{"http:\/\/dx.doi.org\/10.14288\/1.0061624":{"http:\/\/vivoweb.org\/ontology\/core#departmentOrSchool":[{"value":"Science, Faculty of","type":"literal","lang":"en"},{"value":"Chemistry, Department of","type":"literal","lang":"en"}],"http:\/\/www.europeana.eu\/schemas\/edm\/dataProvider":[{"value":"DSpace","type":"literal","lang":"en"}],"https:\/\/open.library.ubc.ca\/terms#degreeCampus":[{"value":"UBCV","type":"literal","lang":"en"}],"http:\/\/purl.org\/dc\/terms\/creator":[{"value":"Xu, Xiaoji","type":"literal","lang":"en"}],"http:\/\/purl.org\/dc\/terms\/issued":[{"value":"2009-05-29T14:28:29Z","type":"literal","lang":"en"},{"value":"2009","type":"literal","lang":"en"}],"http:\/\/vivoweb.org\/ontology\/core#relatedDegree":[{"value":"Doctor of Philosophy - PhD","type":"literal","lang":"en"}],"https:\/\/open.library.ubc.ca\/terms#degreeGrantor":[{"value":"University of British Columbia","type":"literal","lang":"en"}],"http:\/\/purl.org\/dc\/terms\/description":[{"value":"The research work of this Ph.D. thesis is centered on coherent anti-Stokes Raman spectroscopy (CARS) with broad band coherent pulses. After a mathematical derivation of the formula that is responsible for CARS, four new approaches were proposed. The first method of Noise-autocorrelation spectroscopy with coherent Raman scattering utilizes spectral noise to reveal vibrational level spacings through autocorrelation. Its variation of Narrowband spectroscopy by all-optical correlation of broadband pulses, uses the technique of optical processing based on noisy probe pulse of special shape to obtain high resolution CARS spectra. The method of complete characterization of molecular vibration, can measure the phase of laser induced vibration through amplitude and phase retrieval on a time-frequency spectrogram. It is also a high resolution method. The final method Background free coherent Raman spectroscopy by detecting spectral phase of molecular vibrations is the spectroscopic application of detected spectral phase of laser induced vibration.","type":"literal","lang":"en"}],"http:\/\/www.europeana.eu\/schemas\/edm\/aggregatedCHO":[{"value":"https:\/\/circle.library.ubc.ca\/rest\/handle\/2429\/8445?expand=metadata","type":"literal","lang":"en"}],"http:\/\/purl.org\/dc\/terms\/extent":[{"value":"3487495 bytes","type":"literal","lang":"en"}],"http:\/\/purl.org\/dc\/elements\/1.1\/format":[{"value":"application\/pdf","type":"literal","lang":"en"}],"http:\/\/www.w3.org\/2009\/08\/skos-reference\/skos.html#note":[{"value":"New Methods of Coherent Anti-Stokes Raman Spectroscopy Based on Broadband Pulses by Xiaoji Xu B.Sc., Peking University, Beijing, 2004 A THESIS SUBMITTED IN PARTIAL FULFILLMENT OF THE REQUIREMENTS FOR THE DEGREE OF DOCTOR OF PHILOSOPHY in The Faculty of Graduate Studies (Chemistry) THE UNIVERSITY OF BRITISH COLUMBIA (Vancouver) May 2009 c Xiaoji Xu 2009 \u0002 \fAbstract The research work of this Ph.D. thesis is centered on coherent anti-Stokes Raman spectroscopy (CARS) with broad band coherent pulses. After a mathematical derivation of the formula that is responsible for CARS, four new approaches were proposed. The \ufb01rst method of Noise-autocorrelation spectroscopy with coherent Raman scattering utilizes spectral noise to reveal vibrational level spacings through autocorrelation. Its variation of Narrowband spectroscopy by all-optical correlation of broadband pulses, uses the technique of optical processing based on noisy probe pulse of special shape to obtain high resolution CARS spectra. The method of complete characterization of molecular vibration, can measure the phase of laser induced vibration through amplitude and phase retrieval on a time-frequency spectrogram. It is also a high resolution method. The \ufb01nal method Background free coherent Raman spectroscopy by detecting spectral phase of molecular vibrations is the spectroscopic application of detected spectral phase of laser induced vibration. ii \fTable of Contents . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . ii Table of Contents . . . . . . . . . . . . . . . . . . . . . . . . . . . . iii Abstract List of Figures . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . vii . . . . . . . . . . . . . . . . . . . . . . . . . . . . x . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . xi List of Programs Glossary Acknowledgments Dedication . . . . . . . . . . . . . . . . . . . . . . . . . . . xii . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . xiv Statement of Co-Authorship . . . . . . . . . . . . . . . . . . . . . xv 1 Introduction to Coherent Anti-Stokes Raman Scattering . 1.1 1.2 Introduction . . . . . . . . . . . . . . . . . . . . . . . . . . . 1.1.1 Raman E\ufb00ect . . . . . . . . . . . . . . . . . . . . . . 1.1.2 Discovery of Coherent Anti-Stokes Raman Scattering 1 1 1 (CARS) . . . . . . . . . . . . . . . . . . . . . . . . . . 3 1.1.3 Coherent Anti-Stokes Raman Scattering at Glance . . 4 1.1.4 Coherent Spectroscopy 6 1.1.5 Coherent Broad Band Laser . . . . . . . . . . . . . . 7 1.1.6 Pulse Shaping Technique . . . . . . . . . . . . . . . . 9 . . . . . . . . . . . . . . . . . Review on Current Coherent Anti-Stokes Raman Scattering Methods 1.2.1 . . . . . . . . . . . . . . . . . . . . . . . . . . . . . 10 Traditional Narrow Band CARS . . . . . . . . . . . . 12 iii \fTable of Contents 1.3 1.2.2 Multiplex CARS Method . . . . . . . . . . . . . . . . 15 1.2.3 Time-resolved CARS method . . . . . . . . . . . . . . 21 1.2.4 Pulse Shaping in CARS Methods 27 1.2.5 Summary and Comparison of Current Methods . . . 35 Theory of Coherent Anti-Stokes Raman Scattering . . . . . . 37 1.3.1 Brief introduction to Density Matrix 38 1.3.2 CARS Expression Derivation Using Density Matrix Formalism 1.4 . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . 40 1.3.3 Non-resonant Background 1.3.4 Sample Numerical Simulation . . . . . . . . . . . . . 55 1.3.5 Phase Matching Consideration . . . . . . . . . . . . . 57 Experimental Setup and Pulse shaper . . . . . . . . . . . . . 63 1.4.1 Overview . . . . . . . . . . . . . . . . . . . . . . . . . 63 1.4.2 Ti:Sapphire Generative Ampli\ufb01er and OPA . . . . . . 66 1.4.3 Pulse Shaping Techniques . . . . . . . . . . . . . . . . 71 1.4.4 Pulse Characterization 81 1.4.5 Generation and Detection of CARS Signal . . . . . . . . . . . . . . . . . 52 . . . . . . 83 Structure of Ph.D. Thesis . . . . . . . . . . . . . . . . . . . . 85 Bibliography . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . 87 . . . . . 92 . . . . . . . . . . . . . . . . . . . . . . . . . . . . 92 1.5 2 Noise Auto-correlation Spectroscopy with CARS 2.1 Motivation 2.2 Method Content . . . . . . . . . . . . . . . . . . . . . . . . . 103 2.2.1 Content . . . . . . . . . . . . . . . . . . . . . . . . . . 103 2.2.2 Methods . . . . . . . . . . . . . . . . . . . . . . . . . 112 Bibliography . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . 115 3 Narrowband Spectroscopy by All-optical Correlation of Broadband Pulses . . . . . . . . . . . . . . . . . . . . . . . . . . . . . 117 3.1 Motivation . . . . . . . . . . . . . . . . . . . . . . . . . . . . 117 3.2 Experimental Technique Considerations . . . . . . . . . . . . 121 3.3 Method Content . . . . . . . . . . . . . . . . . . . . . . . . . 122 iv \fTable of Contents 3.3.1 Overview . . . . . . . . . . . . . . . . . . . . . . . . . 122 3.3.2 Content . . . . . . . . . . . . . . . . . . . . . . . . . . 122 Bibliography . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . 134 4 Complete Characterization of Molecular Vibrations using Frequency Resolved Gating . . . . . . . . . . . . . . . . . . . 137 4.1 Motivation . . . . . . . . . . . . . . . . . . . . . . . . . . . . 137 4.2 Experiment Technique Considerations . . . . . . . . . . . . . 142 4.3 Method Content . . . . . . . . . . . . . . . . . . . . . . . . . 145 4.3.1 Overview . . . . . . . . . . . . . . . . . . . . . . . . . 145 4.3.2 Content . . . . . . . . . . . . . . . . . . . . . . . . . . 145 Bibliography . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . 155 5 Background-free Coherent Raman Spectroscopy by Detecting the Spectral Phase of Molecular Vibrations . . . . . . . 157 5.1 Motivation . . . . . . . . . . . . . . . . . . . . . . . . . . . . 157 5.2 Method Content . . . . . . . . . . . . . . . . . . . . . . . . . 162 5.2.1 Overview . . . . . . . . . . . . . . . . . . . . . . . . . 162 5.2.2 Content . . . . . . . . . . . . . . . . . . . . . . . . . . 162 Bibliography . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . 170 6 Conclusion . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . 172 Bibliography . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . 177 A MATLAB Simulation code of CARS . . . . . . . . . . . . . . 178 A.1 Generate Pulse A.2 Pulse Shaping . . . . . . . . . . . . . . . . . . . . . . . . . 178 . . . . . . . . . . . . . . . . . . . . . . . . . . 178 A.3 CARS Process Simulation . . . . . . . . . . . . . . . . . . . . 178 A.4 Simulation on XFROG CARS . . . . . . . . . . . . . . . . . 183 v \fTable of Contents Appendices B Alignment of the Pulse Shaper and Calibration of the SLM 185 B.1 Alignment of the Pulse Shaper . . . . . . . . . . . . . . . . . 185 B.2 SLM Voltage to Phase Calibration of CRI-SLM 640 SLM . . 187 C XFROG Retrieval Using FROG3 Software . . . . . . . . . . 191 C.1 Obtaining and formatting the recorded data . . . . . . . . . 191 C.2 Operation with software . . . . . . . . . . . . . . . . . . . . . 192 D New Representations of Characterized Vibrational Coherence . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . 200 D.1 Method Content . . . . . . . . . . . . . . . . . . . . . . . . . 200 Bibliography . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . . 213 vi \fList of Figures 1.1 Energy scheme of spontaneous Raman scattering . . . . . . . 2 1.2 Scheme of coherent anti-Stokes Raman scattering . . . . . . . 5 1.3 Photograph of a pulse shaper . . . . . . . . . . . . . . . . . . 11 1.4 Scheme of narrow band CARS . . . . . . . . . . . . . . . . . 13 1.5 Comparison between Raman and CARS spectrum . . . . . . 16 1.6 Energy scheme of multiplex CARS using a dye laser . . . . . 17 1.7 Setup of a type of multiplex CARS microscopy . . . . . . . . 19 1.8 Microscopy using multiplex CARS . . . . . . . . . . . . . . . 20 1.9 Intensity of multiplex CARS vs. probe bandwidth . . . . . . 22 1.10 Spectrum and its Fourier transform . . . . . . . . . . . . . . . 24 1.11 Time-resolved CARS of hydrogen gas . . . . . . . . . . . . . . 26 1.12 Pulse shape of single pulse CARS . . . . . . . . . . . . . . . . 29 1.13 Numerical simulation on \ufb01eld correlation . . . . . . . . . . . . 32 1.14 Numerical simulation of sinusoidal phase modulated pulse . . 33 1.15 Diagram of CARS . . . . . . . . . . . . . . . . . . . . . . . . 42 1.16 Numerical plot of one resonant level . . . . . . . . . . . . . . 47 1.17 Concept scheme of information \ufb02ow in CARS . . . . . . . . . 51 1.18 Scheme of non-resonant response . . . . . . . . . . . . . . . . 53 1.19 Comparison between shaped pulse and unshaped pulse . . . . 58 1.20 Vibrational coherence and CARS spectra . . . . . . . . . . . 59 1.21 Concept scheme of phase matching in collinear geometry . . 61 1.22 BOXCARS phase matching geometry . . . . . . . . . . . . . 63 1.23 A CARS setup of BOXCARS phase matching geometry . . . 64 1.24 A CARS setup of collinear geometry . . . . . . . . . . . . . . 67 1.25 Scheme of spectral phase pulse shaper . . . . . . . . . . . . . 70 vii \fList of Figures 1.26 Schematic of a spectral phase pulse shaper . . . . . . . . . . . 72 1.27 Optical property of nematic liquid crystal . . . . . . . . . . . 73 1.28 E\ufb00ective refractive index of liquid crystal . . . . . . . . . . . 74 1.29 Scheme of a folded pulse shaper . . . . . . . . . . . . . . . . . 77 1.30 Schematics of a re\ufb02ected folded shaper . . . . . . . . . . . . . 79 1.31 Scheme of FROG device setup . . . . . . . . . . . . . . . . . 82 2.1 CARS signal generation in frequency and time domain . . . . 94 2.2 CARS spectra of chirped pulses and noisy pulses . . . . . . . 95 2.3 The comparison of CARS spectra of di\ufb00erent pulses . . . . . 98 2.4 Single pulse NASCARS time domain representation . . . . . 101 2.5 Energy scheme of CARS and experimental setup . . . . . . . 105 2.6 Energy scheme of noise transformation in both domains . . . 108 2.7 Experimental result of NASCARS . . . . . . . . . . . . . . . 110 3.1 Energy schemes of CARS and SFG . . . . . . . . . . . . . . . 125 3.2 Numerical simulation on the proposed method . . . . . . . . 127 3.3 Scheme of experimental setup . . . . . . . . . . . . . . . . . . 130 3.4 Experiment results of optical correlations . . . . . . . . . . . 131 4.1 Comparison between CARS and SFG 4.2 Numerical comparison between a pure sample and mixture . 140 4.3 Schem of operation steps of XFROG algorithm for CARS . . 143 4.4 Numerical simulation of XFROG method . . . . . . . . . . . 148 4.5 Experimental result of XFROG method . . . . . . . . . . . . 151 4.6 Time domain beating dynamics separation . . . . . . . . . . . 153 5.1 Non-resonant problem using broad band probing . . . . . . . 158 5.2 Spectral phase and total intensity comparison . . . . . . . . . 161 5.3 Comparison between low and high non-resonant background . 165 5.4 Experimental time-frequency trace of azobenzene . . . . . . . 167 5.5 Experiment result 6.1 Other complete characterization scheme . . . . . . . . . . . . 175 6.2 Combination of STIRAP and XFROG . . . . . . . . . . . . . 176 . . . . . . . . . . . . . 139 . . . . . . . . . . . . . . . . . . . . . . . . 168 viii \fList of Figures B.1 Scheme of folded shaper with mirror . . . . . . . . . . . . . . 186 B.2 Calibration illustration of Spatial light modulator . . . . . . . 189 C.1 Step one, functions of software . . . . . . . . . . . . . . . . . 193 C.2 Step two, continue . . . . . . . . . . . . . . . . . . . . . . . . 194 C.3 Step three, input of the probe \ufb01eld \ufb01le . . . . . . . . . . . . . 195 C.4 Step four, noise subtractions . . . . . . . . . . . . . . . . . . . 196 C.5 Step \ufb01ve, resize data . . . . . . . . . . . . . . . . . . . . . . . 197 C.6 Step six, initialize interface . . . . . . . . . . . . . . . . . . . 198 C.7 Step seven, algorithm retrieval . . . . . . . . . . . . . . . . . 199 D.1 Energy diagram and interaction scheme . . . . . . . . . . . . 202 D.2 Experimental CARS spectrogram . . . . . . . . . . . . . . . . 204 D.3 Experimental setup. . . . . . . . . . . . . . . . . . . . . . . . 206 D.4 Shapes of amplitude and phase patterns . . . . . . . . . . . . 207 D.5 Amplitude and phase of retrieved vibrational response . . . . 209 D.6 Calculated spectrograms . . . . . . . . . . . . . . . . . . . . . 211 ix \fList of Programs A.1 MATLAB program that generates E \ufb01eld of a pulse . . . . . 179 A.2 MATLAB program that serves as pulse shaper. . . . . . . . . 180 A.3 MATLAB program that generates CARS. . . . . . . . . . . . 181 A.4 MATLAB program that generates time frequency XFROG trace of CARS . . . . . . . . . . . . . . . . . . . . . . . . . . 183 x \fGlossary BBO \u03b2-Barium Borate CARS Coherent anti-Stokes Raman Scattering CCD Coupled Charge device FROG Frequency Resolved Optical Gating FWM Four Wave Mixing FWHM Full Width at Half Maximum LBO Lithium Triborate MIIPS Multiphoton Intrapulse Interference Phase Scan NASCARS Noise Auto-correlation Spectroscopy with Coherent anti-Stokes Raman Scattering OPA Optical Parametric Ampli\ufb01er PMT Photomultiplier Tube SFG Sum Frequency Generation SHG Second Harmonic Generation SLM Spatial Light Modulator XFROG Cross-correlation Frequency Resolved Optical Gating xi \fAcknowledgments First and foremost, I want to express my cordial thanks to my Ph.D. advisor Dr. John W. Hepburn. As an established chemical physicist, his advice has been the beacon of light guiding me through the whole period of my research. His profound knowledge in spectroscopy, his zeal on research and his kind encouragement inspire me to be a better researcher. I enjoy every discussion with him, for each constructive conversation sparkles new ideas. I want to thank my \u201cde facto\u201d co-advisor Dr. Valery Milner for his extensive advices during my research. He is a truly researcher with both creativity and diligence. Detailed discussions with him and advices from him turn a \ufb02ash of idea into a reality. His high standard on research, meticulous theoretical derivations and numerical simulations drive our experiments towards perfection. I hold deep gratitude to my colleague and coworker, Dr. Stanislav (Stas) O. Konorov. We collaborated on most of experiments presented in this thesis. His knowledge and skill on optics helps me immensely during the experiment. His intrinsic sense of humor always makes a happy experiment even if sometimes experimental results turn out to be negative. I want to express my special thank to Dr. Moshe Shapiro. His course on quantum mechanics at the beginning of my study turned me from an analytical chemistry undergraduate to a chemical physicist. Besides his course, I am greatly bene\ufb01ted from the academic atmosphere of coherent control he has created at University of British Columbia. I would like to thank current and previous members of Hepburn group for the support during my study, the Laboratory for Advanced Spectroscopy and Imaging Research (LASIR) for its state of art research facility and chemistry department of U.B.C. for the teaching assistantship and University Graduate xii \fAcknowledgments Fellowship. xiii \fDedication Dedicate this thesis to my parents and my enlightenment physics teacher, Mrs. Zhou, Shou-Kang, who opened the door of science to me. xiv \fStatement of Co-Authorship This Ph.D. thesis includes several published and in press articles in peerreviewed journals (chapter 2 to 5 and appendix D). I am coauthored in these articles with my supervisors Dr. John W. Hepburn and Dr. Valery Milner, my co-worker Dr. Stanislav O. Konorov, who is a postdoctoral fellow. In all articles in this thesis, I contributed the conception of the idea, played a key role in building all experimental setup, data collections and result analysis. In the article of chapter 4, the pulse shaper used in experiment is built by Mr. Sergey Zhdanovich, a fellow Ph.D. student from the same research group. xv \fChapter 1 Introduction to Coherent Anti-Stokes Raman Scattering 1.1 Introduction 1.1.1 Raman E\ufb00ect The Raman process is a type of inelastic scattering of light which involves the generation of new frequencies during light matter interaction. It was observed by C. V. Raman[1] and independently by Grigory Landsberg and Leonid Mandelstam[2]. Because the generated light frequencies re\ufb02ect the property of the scattering media, Raman scattering is of great signi\ufb01cance for the diagnosis of the chemical composition and structure of molecules. When light is scattered by particles, the majority of photons do not change their frequency, which is elastic and known as the Rayleigh scattering. However in Raman scattering, a small fraction of photons are scattered inelastically, changing their frequency during the light matter interaction. In one type of such scattering, the frequencies of the scattered photons are red-shifted by the energy di\ufb00erence between the ground state and the vibrationally excited states, which is known as Stokes scattering. There is another type of Raman scattering, especially for high temperature samples that have considerable population in the excited vibrational states, the frequencies of the scattered photons are blue-shifted by the energy di\ufb00erence between the ground state and vibrational excited states. It is known as antiStokes scattering.Figure 1.1 shows the energy scheme of these three types 1 \f1.1. Introduction Figure 1.1: This \ufb01gure shows the Stokes scattering, anti-Stokes scattering and Rayleigh scattering 2 \f1.1. Introduction of scattering. Stokes Raman scattering and anti-Stokes Raman scattering are both called spontaneous Raman scattering. In Stokes scattering, the population of the ground state is transferred into excited states, whereas in anti-Stokes scattering the population of excited states is transferred to the ground state. The intensity of spontaneous Raman scattering is linearly proportional to the concentration of the sample and re\ufb02ects the population of energy states. Because the position of vibrationally excited states determines the frequency shift between the incident light and Raman scattered photons, the spectrum of spontaneous Raman therefore has a pro\ufb01le of the energy levels structure of the sample, and the corresponding spectroscopic method is called Raman spectroscopy. Unfortunately, the weak signal of spontaneous Raman constitutes main disadvantage of this method. Sir Raman admitted that Raman e\ufb00ect has \u201cthe excessive feebleness \u201d in his initial article [1]. 1.1.2 Discovery of Coherent Anti-Stokes Raman Scattering (CARS) Light ampli\ufb01cation by stimulated emission of radiation (laser) was achieved \u00af \u00af \u00af \u00af \u00af by Schawlow and Townes [3]. The invention of the laser is a cornerstone for spectroscopy. With the development of high power pulsed laser technology, Maker and Terhune[4] at Ford Motor Laboratory discovered the nonlinear optical process that is now known as Coherent anti-Stokes Raman scattering \u00af \u00af \u00af \u00af (CARS). They used a pulsed ruby laser to systematically investigate third order polarization \u03c7(3) responses of benzene, and among those third order processes was CARS. To do the experiment, they used a Raman cell to generate a frequency-shifted beam, then they combined ruby radiation with the frequency-shifted beam and focused the beams in benzene. A Blue shifted signal was observed. They also discussed the signal ampli\ufb01cation if the energy di\ufb00erence of the beams matching the vibrational levels of the sample. As a result, the spectrum of CARS re\ufb02ects the energy levels of the sample. The \ufb01nal name \u201cCoherent anti-Stokes Raman Scattering\u201d (CARS), which re\ufb02ects the spectroscopic utilization of this process, was given by 3 \f1.1. Introduction Begley et. al. [5]. In the literature, CARS also stands for \u201cCoherent AntiStokes Raman Spectroscopy\u201d. CARS is the nonlinear optical version of Raman scattering: CARS and Raman share the same selection rules[6]; in the ideal case, both yield spectra that correspond to vibrational resonance structures. However CARS gives much higher signal strength (106 times higher)[7] than spontaneous Raman scattering. It is better for those applications that require Raman spectra but the sample is too dispersed to yield a measurable signal. The CARS technique has been widely used for chemical diagnosis, combustion temperature measurement and biological imaging. It is also proven to be useful in remote chemical detection [8, 9], where it is nearly impossible to use spontaneous Raman techniques. The implementation of CARS microscopy by X.S. Xie and coworkers [10] is another signi\ufb01cant achievement for CARS, which enables noninvasive chemical-speci\ufb01c imaging. 1.1.3 Coherent Anti-Stokes Raman Scattering at Glance Under pulsed laser excitation, the CARS process can be conveniently separated into two steps according to the interaction time of the pulses. Figure 1.2 shows the scheme of CARS. During the vibration preparation step, two laser pulses simultaneously arrive at the sample. If the di\ufb00erence between their frequencies covers vibration resonances, a fraction of molecules are excited into vibrationally excited levels. Due to the coherence of laser \ufb01elds, the excited state vibrates \u201ccoherently\u201d with the ground vibration state. The excitation laser with higher frequency is called the pump pulse and the one with lower frequency is called the Stokes pulse. The expression for creating the vibrational coherence has the following form, which will be derived in section 1.3: \u0002 R(\u03a9) = [ v Cv + CnR ] \u00b7 (\u03c9v \u2212 \u03a9) \u2212 i\u03b3v \u0003 Ep (\u03c9)ES\u2217 (\u03c9 \u2212 \u03a9)d\u03c9 (1.1) Where R(\u03a9) is called vibrational coherence function, and it carries the strength of the excitation and re\ufb02ects the pro\ufb01le of the vibrational reso- 4 \fAnti-Stokes W Probe Stokes Pump 1.1. Introduction (v) (g) Figure 1.2: This \ufb01gure shows the scheme of CARS signal generation: coherent vibration excitation by simultaneous arrival of pump and Stokes pulses and coherent scattering of probe pulse at anti-Stokes frequencies of vibrational levels. 5 \f1.1. Introduction nances. Cv ,\u03c9v and \u03b3v are the strength, frequency and line width of vibrational resonant levels, Ep and Es are the pump and Stokes excitation \ufb01elds respectively. The next step is coherent scattering, where a probe pulse interacts with the prepared coherent vibrational level and generates a coherent, directional signal at the anti-Stokes frequency of the probe frequency. The scattered anti-Stokes light carries the information of vibrational coherence and is recorded by a spectrometer. The generation of the CARS signal through probing follows the expression (1.2): ECARS (\u03c9) \u221d \u0003 R(\u03a9)Epr (\u03c9 \u2212 \u03a9)d\u03a9 (1.2) The generation of CARS spectrum is a convolution between the probe \ufb01eld Epr and vibrational coherence function R(\u03a9). Such a convolution plays a central role in the discussion of this thesis. For CARS with a broadband probe pulse, the convolution leads to poor spectral resolution in the CARS spectrum. Methods have been created to recover or partial recover the R(\u03a9) from the CARS spectrum with broad band excitation pulses and they will be discussed. 1.1.4 Coherent Spectroscopy CARS is a typical coherent spectroscopy technique. The technique of coherent spectroscopy is based on either the coherent excitation of atoms and molecules or the superposition of coherent light scattered by molecules and particles [11]. The coherent excitation from laser pulses establishes de\ufb01nite phase relation between the amplitude of the atomic or molecular wave functions. Such a de\ufb01nite phase relation in turn determines the total amplitudes of the emitted, scattered or absorbed radiation. During the excitation step of a coherent spectroscopy, two or more vibrational levels are excited coherently by a coherent broad pulse. The wave functions of the excited levels have \ufb01xed phase relations and can form a wavepacket that propagates in time. In addition, a whole ensemble of many molecules is coherently excited simultaneously to identical level, and such excitation also creates a spatial 6 \f1.1. Introduction distribution of coherent excited molecules. The coherent property constitutes the major di\ufb00erence between CARS and its incoherent counterpart, spontaneous Raman. The coherence between multiple excited levels in the time domain often means the observed CARS signal is also a function of the relative time delay between excitation pulses. In spontaneous Raman, there is no control over time. The time dependence of CARS enables time-resolved CARS studies (see section 1.2.3). The spatial coherence of CARS leads to a directional signal, whereas the signal of spontaneous Raman scattering is distributed over 4\u03c0 steradian solid angle. Such a directional signal bene\ufb01ts the experimental detection of CARS. When the three excitation beams of CARS are placed properly, the generated anti-Stokes signal is automatically separated from the incident beams (see section 1.3.5), and with proper collimating optics, the full intensity of CARS signal can be detected. For the experiment of spontaneous Raman, only a fraction of scattered signal is detected. In terms of the density dependence, the incoherent spontaneous Raman measures the population density of the sample, while CARS has a quadratic dependence on the particle density. In quantum mechanics, incoherent spectroscopy measures the square |\u03c8|2 of the wave function \u03c8, whereas the coherent spectroscopy, such as CARS, is related to wave function \u03c8 itself, therefore yielding additional information on the phase and amplitude [11] (for detail see chapter 4). From the experiment point of view, the preparation of coherently excited levels is best done by a broad band coherent laser, typically a Ti:sapphire femtosecond laser. The de\ufb01nite phase relations between excited vibrational levels also allow the technique of Coherent Control [12] (see below) in coherent spectroscopy. 1.1.5 Coherent Broad Band Laser The implementation of solid state Ti:sapphire femtosecond laser systems [13] in the early 1990s greatly boosted the innovation of CARS methods. The availability of sub 100fs pulses enabled time-resolved CARS experiments, 7 \f1.1. Introduction which were done in the time domain with pump\/Stokes pulses exciting the molecular vibration and a probe pulse checking the excited states after a time delay[14]. The broad bandwidth of the femtosecond excitation pulses enables simultaneously preparation of multiple vibrational levels. The coherent property of the laser \ufb01eld is then transferred to the vibrational levels and a wavepacket is formed. The wavepacket beats in time and generates the detectable anti-Stokes signal when interacting with a probe pulse. Fourier transform is then used to convert the time domain vibrational beatings to the vibrational level spacing. In addition to the availability of direct time domain research, femtosecond lasers with the high peak intensity leads to high signal strength in the CARS signal. For example, given the same average output power, the 100fs Ti:Sapphire regenerative laser system has 100 times higher peak power than that of 10ps Nd:YAG of same repetition rate. The femtosecond laser has 104 times higher total CARS signal than that from the Nd:YAG laser. Femtosecond laser systems also provide a more convenient frequency conversion than the Nd:YAG laser pumped dye lasers. The optical parametric ampli\ufb01er (OPA) used with Ti:Sapphire femtosecond laser can provide frequency conversion from a wavelength of 300nm to 2000nm. In terms of e\ufb03ciency, an OPA can convert about 25% of the input light into tunable light. Wide range tunability facilitates CARS studies. With an OPA, the CARS experiment can conveniently work with three separate frequencies as pump, Stokes and probe pulses, and this adds \ufb02exibility to the experiment. For example, pulse shaping can be done independently on the three pulses, and the relative time delay between probe and the pump\/Stokes pair can be adjusted as well. From a broader perspective, the broad bandwidth of the Ti:Sapphire laser also enables an easy way to implement the coherent control technique. Coherent control is a family of quantum mechanical based methods that use quantum interference of two or more di\ufb00erent pathways to control the \ufb01nal state of dynamic processes controlled by light \ufb01elds. The general concept was \ufb01rst proposed in 1986 by P. Brumer and M. Shapiro [15]. Numerous experiments [16] have been done in coherent control, such as controlling 8 \f1.1. Introduction the direction of electron motion in semiconductors [17], and the breaking of chemical bonds [18]. Femtosecond Ti:Sapphire laser pulses come with a broad bandwidth and de\ufb01nite spectral phase which can be used to construct the multiple pathways required in coherent control. Control of chemical reactions by feedback-optimized phase-shaped femtosecond laser pulses was demonstrated by G. Gerber and colleagues [19], where the spectral phase of a broad band coherent pulse was pulse shaped to control the outcome of organometallic photo-dissociation reactions. A comprehensive discussion of coherent control can be found in the book \u201cPrinciples of the Quantum Control of Molecular Processes\u201d by M. Shapiro and P. Brumer [12]. In the actual CARS experiments of this thesis, the concept of coherent control heavily in\ufb02uenced the way the experiment was done and particularly, the way that pulse shaping technique was used, even though the experiments per se were not done for the aim of applying coherent control or a new demonstration of coherent control technique in CARS. 1.1.6 Pulse Shaping Technique Because femtosecond lasers possess a broad bandwidth, the phase of spectral components across the bandwidth can have di\ufb00erent values. Spectral phases across the broad band pulse now become a controllable parameter in CARS experiments. The pulse shaping technique[20] is a powerful tool to control the spectral phase as well as the amplitude of the pulse. Pulse shaping is done through an assembly of optical devices collectively called a pulse shaper, as shown in \ufb01gure 1.3. In a pulse shaper, the input pulse is spectrally dispersed into frequency components by a grating. Then the frequency components are collimated by a lens and passing through a spatial light modulator (SLM). The amplitude and spectral phase of each frequency components are controlled independently according to each pixel of the SLM (for detail see section 1.4.3). An exact replica of the lens and the grating is used to reconstruct the dispersed light into a pulse and give an output. The pulse shaper controls the amplitude and phase of light in the frequency domain. Because the frequency and time domain response of a broad band 9 \f1.2. Review on Current Coherent Anti-Stokes Raman Scattering Methods pulse is linked by Fourier transform, the phase and amplitude manipulation in the frequency domain also leads to the full pro\ufb01le control in the time domain. Controllable chirp or a train of small pulses can be created from a coherent broad band pulse with a pulse shaper. In CARS, the pulse shaping technique has been used to improve spectral resolution [21] and selectively excite one resonance from serval adjacent levels[22]. The state-of-the-art pulse shaping technique also enables single pulse CARS techniques. By properly tailoring a single broadband pulse, di\ufb00erent frequency components can serve as pump, Stokes and probe pulse respectively and generate the CARS signal[23, 24]. The following sections 1.2 to 1.4 provide a detailed background knowledge to CARS. Section 1.2 gives a review of the literature. It brie\ufb02y describes the development of CARS methods and discusses respective strengths and weaknesses of current methods. In section 1.3, the analytical expression for CARS signal generation is derived using the time domain representation. The discussion of the e\ufb00ect of non-resonant background and requirement of phase matching is presented. section 1.3 also includes a numerical simulation of CARS signal. In section 1.4, the experimental techniques are discussed. The Ti:Sapphire laser and OPA are described. A detailed recipe for construction of a pulse shaper is included as well as some useful tips for CARS signal generation. 1.2 Review on Current Coherent Anti-Stokes Raman Scattering Methods A review of current CARS techniques and applications can help readers understand the background of this thesis work. Since the discovery of coherent anti-Stokes scattering, CARS techniques have been widely used for various applications from chemical and combustion diagnosis to biological imaging. Understanding the mechanism, strengths and weaknesses of each CARS method can provide guidance to the research of this thesis. For the convenience of discussion, CARS methods are categorized into 10 \f1.2. Review on Current Coherent Anti-Stokes Raman Scattering Methods A B f f lens grating input pulse f f lens grating spatial light modulator shaped pulse (SLM) Figure 1.3: (A) shows a photograph of a pulse shaper. (B) shows the scheme of optical elements. f is the focal length of the lenses. 11 \f1.2. Review on Current Coherent Anti-Stokes Raman Scattering Methods two types in this thesis discussion: frequency domain methods and time domain methods. The initial CARS discovery and development used frequency domain methods. The equipment was based on narrow band laser systems and the purpose of the spectroscopy was to resolve the resonances of the sample. Later, especially after the invention of solid state femtosecond lasers, time domain methods became common in the chemical physics community. Time domain methods are capable of investigating the time dynamics of excited resonant states, and through Fourier transform, giving the spectroscopic information on level spacings and lifetimes. The solid state femtosecond laser also provides coherent broad band pulses which can be used to access multiple resonances in frequency domain methods. 1.2.1 Traditional Narrow Band CARS The Coherent anti-Stokes Raman scattering e\ufb00ect was \ufb01rst observed by Maker and Terhune[4] in 1965. Their experiment was done with a ruby laser system with 100mJ per pulse of 30 ns duration. The output pulse of the ruby laser was guided through a cell \ufb01lled with benzene to generate a frequency shifted beam through stimulated Raman emission. Then the generated beam interacted with ruby radiation again and generated the antiStokes frequency signal from the same benzene sample. Retrospectively, this experiment was a milestone for the CARS spectroscopy. However, the lack of tunable laser sources at that time limited its real spectroscopic applications. With the development of tunable dye laser sources [25], CARS spectroscopy developed considerably during 1970s [26] from the original Maker and Terhune experiment. It became a very attractive method in the \ufb01eld of chemical diagnosis, particularly in situations where normal spontaneous Raman gives very low signal or high background, such as fuel combustion. During this period, besides the task of obtaining spontaneous Raman equivalent spectra, one major application of the CARS method was to measure the temperature of combustion. This involved of the measurement rotational lines intensities with good spectral resolution, and calculation of gas temperatures through the rotation state partition function. 12 \f1.2. Review on Current Coherent Anti-Stokes Raman Scattering Methods Figure 1.4: (A) shows the energy diagram for CARS. (B) shows a typical experimental setup of narrow band CARS. The spectrum is obtained through scanning the frequency of the dye laser system. In this setup, the pump pulse also acts as probe. 13 \f1.2. Review on Current Coherent Anti-Stokes Raman Scattering Methods The typical frequency domain CARS experiment utilizes two laser frequencies to generate detectable CARS signal at the anti-Stokes frequency as \ufb01gure 1.4A shows. A typical setup includes a frequency doubled Nd:YAG laser pumping a dye laser to provide frequency tunable output. One laser frequency from either the Nd:YAG laser or dye laser serves as both pump and probe beam, the other serves as the Stokes beam. To obtain a CARS spectrum, the frequency of the dye lasers is scanned and the CARS signal intensity is recorded as a spectrum. A spectrometer with a photomultiplier tube (PMT) detector is often used to detect the weak CARS signal. During 1970s to 1980s, CARS spectroscopy was treated as an extension of traditional Raman spectroscopy. The theoretical discussions on CARS were presented in the context of nonlinear optics. In nonlinear optics, CARS is treated as a type of resonant four-wave-mixing. The signal is described by the phenomenological third order susceptibility \u03c7(3) by Eas \u221d \u03c7(3) Es\u2217 Ep2 (1.3) The Eas is the anti-Stokes \ufb01eld and Ep and Es are the input \ufb01elds of pump and Stokes pulse respectively, with frequencies at \u03c9pu and \u03c9S . The \u03c7(3) has two parts, the resonant part \u03c7R and non-resonant part \u03c7nR (see below). When the frequency di\ufb00erence between pump and Stokes matches a resonance, the value of di\ufb00erential Raman cross-section d\u03c3\/d\u03a9 is related to the resonant part of \u03c7(3) by expression:[5] \u03c7R = \u03c0c4 d\u03c3 h\u0304\u03c9pu \u03c9s3 \u0393 d\u03a9 (1.4) with \u0393 being the linewidth of the resonant level. \u03c7(3) can be experimentally measured by recording energies of CARS signal and input pump\/Stokes beams [5]. Experiments were carried to measure the Raman cross-section of methane [27, 28]. Because lasers can probe samples non-invasively and are capable of penetrating very high temperature gas samples, CARS has been used in combustion investigations [29, 30] and plasma probing [31]. CARS thermometry 14 \f1.2. Review on Current Coherent Anti-Stokes Raman Scattering Methods [32, 33] was developed to measure the temperature of rapidly \ufb02owing gas. This method relies on the rotational line intensities in the high resolution CARS [34, 35] spectrum. The intensity of rotational lines re\ufb02ects the population of that rotational level. The rotational population can be used to extract the gas temperature T through a calculation involving the Boltzmann distribution equation: 2j1 + 1 \u0394E\/(kB T ) N1 = e N2 2j2 + 2 (1.5) with N1 \/N2 being the population ratio of two rotational lines and \u0394E being the energy di\ufb00erence between two rotational levels. j1 and j2 are the rotational quantum number of rotational states. This technique was used in the diagnosis of internal combustion engine [36, 37] and monitoring of jet engine exhaust [38]. It should be noted that peak positions in CARS are sometimes shifted from the vibrational resonances due to the presence of non-resonant background. The non-resonant background of CARS is from the non-resonant four-wave-mixing of the pump and Stokes pulses and does not re\ufb02ect the pro\ufb01le of the vibrational resonance. Because the resonant CARS signal and the non-resonant background are both coherent, they optically interfere and lead to a distorted CARS spectrum of dispersion pro\ufb01les. Figure 1.5 shows the comparison between the pro\ufb01le of CARS with non-resonant background and the pro\ufb01le of vibrational resonances. Additional \ufb01tting procedures are often required for data interpretation of CARS spectra with non-resonant background [39, 40]. Detailed discussion on the origin of non-resonant background will be discussed in section 1.3.3. 1.2.2 Multiplex CARS Method Measuring spectra from turbulent gases in combustion requires faster measuring speed than that from a stable gas phase sample. The narrow band CARS methods described in the previous section requires scanning of one laser frequency, which is time consuming. Researchers need a fast method to 15 \f1.2. Review on Current Coherent Anti-Stokes Raman Scattering Methods Figure 1.5: This numerical simulation \ufb01gure shows the comparison between the CARS spectrum with non-resonant background (blue line) and pro\ufb01le of vibrational resonances (red dashed line). There are two resonances at 980 and 1040cm\u22121 in the simulation. The strength of the non-resonant background equals 30% of the intensity of the 1040cm\u22121 peak. When the non-resonant background is present, the CARS spectrum shows shifted peak position with a dispersive pro\ufb01le due to interference between resonant signal and non-resonant background. 16 \f1.2. Review on Current Coherent Anti-Stokes Raman Scattering Methods Anti-Stokes Probe Stokes Pump Figure 1.6: This \ufb01gure schematically shows the energy scheme of multiplex CARS using one narrow band laser as pump and probe, and a broad band pulse as Stokes. The narrow band pump and broadband Stokes pulses excite multiple resonant states simultaneously, and excited states are probed by the narrow band probe pulse to give multiplex CARS spectrum. Dye lasers are used for the broad band Stokes pulse in early experiments. Then solid state broad band lasers later replaced dye lasers as broad band light source for multiplex CARS applications. 17 \f1.2. Review on Current Coherent Anti-Stokes Raman Scattering Methods obtain high resolution spectra without tuning the frequency of the laser. The invention of multiplex CARS [41] satis\ufb01ed such a need. Multiplex CARS is associated with broad band lasers, which may not necessarily be coherent. The idea is to use broadband pulse(s) to excite multiple levels and simultaneously \u201cread out\u201d the CARS spectrum. The early multiplex CARS was done using modeless dye lasers [42], where a Nd:YAG laser pumped dye laser gives broad band incoherent radiation. This broad band emission serves as the Stokes pulse and a narrow band frequency doubled Nd:YAG pulse serves as the pump and probe pulse in CARS. The \ufb01eld correlation between the narrow band pump and the broad band Stokes pulse has broad frequency bandwidth and can simultaneously cover multiple levels. When the probe pulse has narrow bandwidth, the CARS spectrum is a replica of the pro\ufb01le of the prepared ro-vibrational levels without frequency scanning. Figure 1.6 shows the energy scheme of one multiplex CARS method. Because of the ability to read out the rotational CARS spectrum in one shot, multiplex CARS further improved gas temperature measurement[43\u2013 46] for combustion diagnosis and temperature measurement. For the multiplex CARS method shown in \ufb01gure 1.6, the bandwidth of the Stokes determines the vibration resonance \u201cread out\u201d window and the narrowness of the probe pulse determines the spectral resolution. Multiplex CARS has been gaining strength with the development of laser technologies. The invention of solid state Ti:Sapphire lasers [13, 47, 48] greatly improved the application of the CARS method. The ampli\ufb01ed Ti:Sapphire laser can conveniently provide 35fs duration broad band pulses of 450cm\u22121 bandwidth centered around 800nm wavelength. Ti:Sapphire lasers are more stable and easier to maintain than organic dye lasers. With the broad bandwidth, it becomes feasible to create a narrow band probe pulse from broad band radiation. In Prince et. al. [49], grating pairs are used to create a pulse of about 10cm\u22121 bandwidth from a broad band pulse, and the created narrow band pulse is used as the probe pulse in CARS. An important application of multiplex CARS is the microscopy of living cells (see works of Cheng et.al. [50] and Mu\u0308ller et.al.[51]). In these experiments, a picosecond laser system is synchronized with a femtosecond 18 \f1.2. Review on Current Coherent Anti-Stokes Raman Scattering Methods Figure 1.7: This \ufb01gure shows a schematic of the experimental setup for multiplex CARS microscopy. Two laser systems, a 10 ps and a 80 fs modelocked Ti\/sapphire lasers were used to provide narrow band pump and broad band Stokes pulses. Microscope objectives O1 ,O2 were used to focus and collimate the beams ; Signal generated from sample (S) was \ufb01ltered by a band pass \ufb01lter. The laser pulses from the two lasers were actively synchronized. (from M. Mu\u0308ller et. al. J. Phys. Chem. B 2002, 106, 3715-3723) 19 \f1.2. Review on Current Coherent Anti-Stokes Raman Scattering Methods Figure 1.8: This \ufb01gure shows multiplex CARS image of a multi-lamellar vesicle using the 1128cm\u22121 resonance. The acquisition time per pixel was 200 ms, and the image has 50 \u00d7 50 pixels. The insets show the CARS spectrum of the lipids (a) and the surrounding water (b).(from M Mu\u0308ller et. al. J. Phys. Chem. B 2002, 106, 3715-3723). Ti:Sapphire laser to provide pump and Stokes pulses for CARS excitation. Figure 1.7 schematically shows the setup. With a tight beam focus using a high numerical aperture microscope objective[10] to satisfy the phase matching condition (details see section 1.3.5), the pump and the Stokes pulses generate a CARS spectrum inside living cells. In Cheng et.al [50], the spectrum of cellular lipids was obtained. By scanning the focus spot across di\ufb00erent parts of the cell, an image of three-dimensional distributions of cellular lipids was measured and reconstructed. In the work of Mu\u0308ller et.al.[51], the image of a multi-lamellar vesicle was obtained by multiplex CARS microscopy as shown in \ufb01gure 1.8. Multiplex CARS microscopy has the potential of obtaining the spectrum when doing imaging, therefore providing better information on chemical-speci\ufb01c distributions. The major 20 \f1.2. Review on Current Coherent Anti-Stokes Raman Scattering Methods challenge for multiplex CARS microscopy is its acquisition time. For example, an image of 100 \u00d7 100 pixels has 104 points. If the exposure time of CCD for one spectrum can be as fast as 20ms, the total acquisition time for one image is 200s. It is hard to obtain a realtime image with CARS. In the work of Mu\u0308ller et.al.[51], each pixel took 200ms to acquire. Faster detectors can improve the performance. In the work of Cheng et.al. [50], a PMT dector is used to reduce the acquisition time. For the particular experiment setup that requires synchronization between two lasers [50, 51], time synchronization between a femtosecond laser system and a picosecond laser system requires special feedback control system and susceptible to instability [52]. Multiplex CARS is an improvement on narrow band CARS methods because of its ability to obtain CARS spectra without scanning the frequency of the excitation laser. It dramatically reduces the measurement time of CARS. However, multiplex CARS still su\ufb00ers from two major disadvantages: \ufb01rstly, the spectral resolution is limited by the bandwidth of the probe pulse, as the CARS spectrum is still a frequency domain convolution between pro\ufb01les of vibrational resonances and the probe bandwidth. Secondly, from the signal strength point of view, a narrow band pulse coming with a low peak power yields less signal in a nonlinear process such as CARS. Figure 1.9 shows the numerical comparison between signal strength from probe pulses of di\ufb00erent bandwidth cut from the same broad band source: 100cm\u22121 (thick blue), 10cm\u22121 (dashed green) and 1cm\u22121 (thin red). Trimming the bandwidth from 100cm\u22121 to 1cm\u22121 reduces the total intensity by approximately two orders of magnitude. 1.2.3 Time-resolved CARS method In the early 1980s, scientists successfully brought down the duration of laser pulses into the femtosecond range using dye laser systems [53]. The later discovery of the solid state Ti:Sapphire laser[13] in the early 1990s further shortened the pulse duration to even sub 10fs and greatly ampli\ufb01ed the pulse power. A typical commercially available Ti:Sapphire laser system can con- 21 \f1.2. Review on Current Coherent Anti-Stokes Raman Scattering Methods x1 10 8 x4 6 x40 4 2 0 720 730 740 750 760 770 wavelength (nm) Figure 1.9: This \ufb01gure shows the CARS signal intensity comparison between di\ufb00erence bandwidth of the probe pulses. Probe pulses have the same spectrum peak intensity. The CARS spectrum using a raw 100cm\u22121 transform-limited bandwidth probe pulse (thin blue line), the CARS spectrum using a probe pulse of 10cm\u22121 bandwidth, trimmed from the raw 100cm\u22121 pulse (red thick line) and the CARS spectrum using a probe pulse of 1cm\u22121 bandwidth, trimmed from the raw 100cm\u22121 pulse (green dashed line). Two vibrational levels are used in this simulation. 22 \f1.2. Review on Current Coherent Anti-Stokes Raman Scattering Methods veniently provide below 100fs radiation. The availability of short duration pulses has facilitated the temporal domain investigation of CARS. With femtosecond duration laser pulses from dye lasers, Zewail and his colleagues pioneered the \ufb01eld of femtochemistry[54]. Their work on ultrafast dynamics contributed to the \ufb01eld of time domain spectroscopy and caught the attention of the scienti\ufb01c community. By means of coherent ultrafast lasers, temporal domain molecular coherence was revealed and interpreted. Through a series of pump\/probe experiments, it was shown that the temporal domain vibrational wave packet can as well re\ufb02ect the vibration spacing through means of Fourier transform [55\u201357]. \u201dPump\/probe\u201d is the most commonly used scheme in femtochemistry: a broad band coherent pump pulse excites the molecular system, preparing a wave packet, and a second pulse coming after a variable delay probes the prepared system. Time-resolved CARS can be treated as a generalized \u201cpump\/probe\u201d experiment. The function of the pump\/Stokes pulse pair can be regarded as the \u201cpump\u201d, and the probe pulse in CARS serve as the \u201cprobe\u201d. In CARS, the simultaneous interaction of pump and Stokes pulses prepares a Raman wave packet. The subsequent probing pulse generates CARS signals that re\ufb02ect the propagation of the prepared vibrational wave packet. Figure 1.2 schematically depicts such a process. In the experimental realization, a timeresolved CARS experiment utilizes three broadband femtosecond excitation pulses. Short duration pump and Stokes pulses overlap in time followed by a probe pulse with variable time delay, and the modulation of CARS signal is recorded. After obtaining the CARS signal vs. time delay response, a Fourier transform is used to obtain the resonance spacing in the frequency domain. Figure 1.10 (B) and (D) shows the simulation of vibration beating of toluene and its Fourier transform revealing the vibrational level spacing. The Time-resolved CARS method was used initially to investigate the dephasing of vibrational levels [58, 59]. Dephasing of vibrational levels leads to a decrease of CARS signal and provides insight into molecular structure and its solvent environment [60]. The direct time domain measurement can provide more accurate data on the time domain behavior of dephasing, comparing to linewidth methods. The spectral resolution of the narrow band 23 \f1.2. Review on Current Coherent Anti-Stokes Raman Scattering Methods 0.5 (B) (A) 0.4 6000 0.3 4000 0.2 2000 0.1 0 650 0 750 850 950 1050 1150 \u22121 Wavenumber (cm ) 0 2000 4000 6000 8000 Time (fs) 11 x 10 20000 (D) (C) 4 15000 10000 2 5000 0 0 \u22122000\u22121000 0 1000 2000 Time (fs) \u2212300\u2212200\u2212100 0 100 200 300 \u22121 Wavenumber (cm ) Figure 1.10: (A) shows a simulation of the vibrational spectrum of toluene with resonances at 782cm\u22121 ,1000cm\u22121 and 1027cm\u22121 . (B) shows the simulation of time domain beating of toluene excited by 100fs pump and Stokes pulses with a frequency di\ufb00erence centered at 900cm\u22121 . (C) shows the direct Fourier transform of the spectrum in (A). (D) shows the Fourier transform of the time domain beating in (B) 24 \f1.2. Review on Current Coherent Anti-Stokes Raman Scattering Methods CARS method limits the accuracy of the linewidth measurement. For example, if the probe pulse bandwidth is 0.5cm\u22121 , when measuring an energy level with 1cm\u22121 linewidth, the error on the lifetime is quite high due to spectral resolution (5.3 ps for 1cm\u22121 , comparing to 3.5ps for 1.5cm\u22121 ). On the other hand, the error associated with direct measurement in the time domain is only limited by the duration of the probe pulse, which is often sub 100fs in typical time-resolved CARS experimental setup. When multiple levels exist within the excitation bandwidth [61], a vibrational wave packet is prepared and resonant level spacing can be calculated through the Fourier transform of the vibrational beating. Time resolved CARS can also be used to perform temperature and pressure measurements. Motzkus and coworkers performed a time resolved CARS experiment on H2 gas [62]. The experimental signal showed detailed beating behavior in the time domain, re\ufb02ecting the rotational dynamics of all thermally populated rotational levels. Modeling of the experimental time domain response gave the temperatures of the gas (see \ufb01gure 1.11). Time-resolved CARS is the temporal domain counterpart to the previously discussed frequency resolved methods. The high peak power of ultrafast pulses used in time resolved CARS gives high signal strength. When recording the beating response, it does not require high resolution spectrometer, and the method is capable of detecting dilute gas samples because of high signal strength. The core of this method is to obtain the vibrational beating and perform Fourier transform to obtain resonance spacing information. However, the reliance on Fourier transform leads to an underlying problem. Time domain CARS beating measurements and frequency domain CARS spectra are not equivalent [63]. The Fourier relations between spectra, vibrational beating and their corresponding Fourier transforms are compared in \ufb01gure 1.10. It shows that the fourier transform of vibrational beating does not equal the spectrum and vice versa. The Fourier transform of time domain beatings (\ufb01gure 1.10B) gives a symmetrical frequency domain response (\ufb01gure 1.10D) which is di\ufb00erent from the actual spectrum of vibrational resonances (\ufb01gure 1.10A). The Fourier transform of the fre25 \f1.2. Review on Current Coherent Anti-Stokes Raman Scattering Methods Figure 1.11: (A) Time resolved CARS signal of H2 gas at four di\ufb00erent temperatures. (b) Rotational level populations can be calculated through \ufb01tting. (from T. Lang et. al. Phys. Chem. Lett. 1999, 310, 65-72) 26 \f1.2. Review on Current Coherent Anti-Stokes Raman Scattering Methods quency domain spectrum \ufb01gure (\ufb01gure 1.10A) gives symmetric time domain pro\ufb01les (\ufb01gure 1.10C), which is contradictory to the direct time domain beating measurement. This is a problem of the Fourier transform in linking experimental results of the time domain to the frequency domain and vice versa. The reason this problem exists is the lack of phase information in the measurement. Photon detectors, such as a PMT, or a CCD cannot record the phase of the optical \ufb01eld, only records the intensity of the \ufb01eld, which is the modulus square of \ufb01eld amplitude. The Fourier transform of a real quantity from experimental measurement gives a symmetric response in the conjugated domain. However, if the phase factor is considered into the Fourier transform, the complex spectrum will be equivalent to the vibrational beating, and the Fourier transform of beating signal with phase will give the actual CARS spectrum. This raises the question of how to obtain the phase of vibrational responses. In chapter 4, a tentative approach will be presented. 1.2.4 Pulse Shaping in CARS Methods Beside having a broad bandwidth, Ti:Sapphire lasers also provide coherent broad band radiation. The concept of coherence describes the correlation properties between physical quantities of a wave. Spectral components in broad band coherent radiation maintain stable phase relations. This is the fundamental di\ufb00erence between a femtosecond Ti:Sapphire laser and a modeless dye laser: a dye laser gives a sum of shifting spectral lines within bandwidth from shot to shot, while a Ti:sapphire laser gives a stable broadband output every shot. Such stable qualities of both amplitude and spectral phase of coherent lasers lead to the possible utilization of interference e\ufb00ects. To manipulate the spectral phase of a broad band pulse, the technique of pulse shaping is often implemented to control interference e\ufb00ect. The functions of the pulse shaping technique in CARS can be categorized into two types. In the \ufb01rst type, the pulse shaper tailors broad band spectral components to ful\ufb01l the vibrational excitation task and the probing task. It is primarily used for single pulse CARS experiments. In the second type, the 27 \f1.2. Review on Current Coherent Anti-Stokes Raman Scattering Methods pulse shaper controls the phase and sometimes the amplitude of excitation pulse pairs or the probe pulse to achieve selective excitations or selective probing. Single Pulse CARS method Single pulse CARS utilizes the pulse shaping technique on broad band radiation to include the vibrational excitation and coherent probing within one broad band pulse. The preparation of molecular vibrations through a single broad band femtosecond pulse is known as impulsive stimulated Raman scattering [64, 65]. Impulsive stimulated Raman scattering was used for vibrational excitation in a single pulse CARS method. Due to the broad bandwidth of femtosecond pulses, if the frequency di\ufb00erence between the red edge and the blue edge of a pulse coincides with a vibration resonance of sample, a vibrational coherence is prepared. The impulsive stimulated Raman process can be treated as a special case of coherent stimulated Raman with a single pulse acting as both pump and Stokes pulses. The amplitude and phase control ability of the pulse shaper is used to include the probe function into one single broad band pulse. A narrow band spectral component at the blue edge of the spectrum is shaped with di\ufb00erent spectral phase from the rest of the spectrum to serve as the probe pulse. The pulse shaping of such a broad band pulse is shown in \ufb01gure 1.12. It was \ufb01rst demonstrated by Y. Silberberg and coworkers [21]. The pulse shaper blocks the blue edge of broad band spectrum using an amplitude mask. The function of this amplitude mask is to remove the potential spectral overlap between the excitation pulse and the generated CARS signal. Then, at the remaining blue edge of the spectrum, a spectral phase shift is applied to a narrow window of the spectrum. This out of phase spectral component serves as the function of probe pulse, because in the time domain it corresponds to a long time duration. The pulse after the pulse shaper was then focused by a high numeric aperture microscope objective at the sample to generate CARS signals in the collinear geometry. With proper bandpass 28 \f1 5 Probing part Excitation part 4 3 2 Phase Amplitude (AU) 1.2. Review on Current Coherent Anti-Stokes Raman Scattering Methods 1 0 0 790 795 800 805 810 815 820 825 -1 Amplitude (AU) wavelength (nm) 1 Excitation part Probing part 0 0 0.2 0.4 0.6 0.8 1 1.2 Time (ps) Figure 1.12: The pulse shape of the excitation pulse in single pulse CARS experiment is shown in these plots. The upper plot is the frequency domain representation of broadband pulse amplitude and spectral phase. The narrow spectral phase \ufb02ipped region serves as the probe pulse. The \ufb02at phase region serves as the excitation part. The bottom plot shows the time domain plot of the pulse. 29 \f1.2. Review on Current Coherent Anti-Stokes Raman Scattering Methods \ufb01lters to remove the excitation pulse, the CARS signal was then coupled into a spectrometer to give the spectrum. In Oron et. al. [21], the spectral phase shift of the probing spectral component was set alternatively to \u03c0 and 0. The di\ufb00erence between CARS spectra from these two phase patterns was recorded and the resonant level positions of sample were obtained. In continuing work of Y. Silberberg and coworkers [23] and S.R. Leone and coworkers [24] this method was further developed by introducing heterodyne and polarization techniques for detection. The bandwidth of the femtosecond pulse after shaping usually determines the bandwidth of resonances that single pulse CARS methods can detect. In Lim et. al.[24], a 11fs Ti:sapphire oscillator was used and the measurable spectral range was from 400 to 1500cm\u22121 . The lower range is determined by the e\ufb03ciency of spectral \ufb01ltering, background subtraction as well as the probe pulse band width. The upper limit is determined by the total pulse bandwidth. The resolution of the single pulse CARS method is determined by the width of the probe phase window, and phase window size is limited by the pulse shaper resolution. In Lim et. al.[24], two pixels of the pulse shaper were used to create the probe phase window, and the resulting resolution was about 35cm\u22121 . Reducing the size of the probe window can give better spectral resolution at the cost of signal strength. Single pulse methods have the edge over traditional CARS methods in a way that it greatly simpli\ufb01es the experimental setup. Comparing to traditional requirement of multiple laser frequencies, the single pulse CARS method requires only a femtosecond oscillator, a pulse shaper and a spectrometer. It also removes the time and e\ufb00ort on beams temporal synchronization and spatial overlap. The acquisition speed of the single pulse CARS technique can be shortened to milliseconds as well, since it is only limited by the response time and sensitivity of CCD detector. Selective Excitation through Pulse Shaping With the utilization of pulse shaping, selective preparation of vibration resonances within the excitation bandwidth became a possibility. In the narrow 30 \f1.2. Review on Current Coherent Anti-Stokes Raman Scattering Methods band CARS method, vibrational state selection is done by tuning the frequency of excitation lasers. Frequency tuning of a narrow band laser means long operation time and possible instrument instability. Pulse shapers can manipulate the frequency components within the bandwidth of laser. It enables the possibility of fast selection of vibration excitation without tuning the laser frequency. An early experiment of bandwidth selectivity on the CARS excitation was done through chirping. Chirp is a special phenomenon associated with ultrafast laser pulses. Due to the linear dispersion of light transmitting media, ultrafast pulses extend in duration along the propagation direction. Usually, red frequency components travel faster than blue frequency components in normal dispersion media. If such a chirped pulse is shone on a sample, the low frequency part will arrive earlier than the high frequency part. Hence, the instantaneous frequency that the sample feels gradually shifts toward higher frequency. Such frequency shifting resembles a bird\u2019s chirp in an acoustic wave, so it is given the name \u201cchirp\u201d. Mathematically, a chirped pulse has a quadratic spectral phase dependence on frequency and can be accurately created by a pulse shaper. The special property of time-frequency dependence of a chirped pulse enables a way of controlling the excitation bandwidth of vibrational excitation. For pump and Stokes pulses, if either one is chirped, by varying the time delay between two pulses, the central frequency of the \ufb01eld correlation will shift accordingly. Figure 1.13 is a numerical simulation of the frequency correlation between two chirped pulses. It can be seen that by tuning the relative time delay between pulses, the selection of instantaneous frequency of coherent vibration excitation is achieved. One selective excitation scheme based on chirp was proposed by Zheltikov and coworkers[66] and experiment was done later by Pestov et al.[67] on a solid power sample. Chirp is not the only way of vibrational selection. Any pulse shaping that can a\ufb00ect the spectrum of pump\/Stokes \ufb01eld correlation has the potential of selective excitation . Silberberg and his coworkers explored shaping based on single pulse impulsive Raman process[22, 68]. In their work, sinusoidal 31 \fAmplitude 1.2. Review on Current Coherent Anti-Stokes Raman Scattering Methods t (A) Time delay between pulses Convolution frequency cm -1 400 (B) 600 800 1000 1200 1400 1600 1800 -500 -400 -300 -200 -100 0 100 200 300 400 500 Time delay between pulses (fs) Figure 1.13: (A) schematically shows the overlapping between two chirped pulses in the time domain; \u03c4 is the time di\ufb00erence between center of pulses. (B) shows the numerical simulation of the instantaneous frequency of \ufb01eld correlation. We can see that the convolution frequency now has narrow bandwidth and is a function of relative time delay \u03c4 between pulse and Stokes pulse. 32 \f1.2. Review on Current Coherent Anti-Stokes Raman Scattering Methods 9 x 10 Amplitude (AU) \u22121 (A) 2 150 cm \u22121 200 cm \u22121 250 cm 1.5 1 0.5 0 \u22121000 \u2212800 \u2212600 \u2212400 \u2212200 0 Time (fs) 200 400 600 800 4 x 10 \u22121 Amplitude (AU) 8 150 cm \u22121 200 cm 250 cm\u22121 (B) 6 4 2 0 0 50 100 150 200 250 \u22121 Convolution frequency (cm ) 300 350 400 Figure 1.14: The \ufb01gures show the numerical simulation of femtosecond pulse under sinusoidal spectral phase modulation of 150, 200 and 250 cm\u22121 period. (A) shows the pulse train in the time domain with spectral phase sinusoidal period of 150, 200 and 250cm\u22121 respectively. (B) shows the frequency domain convolution \ufb01eld spectrum. We can see 150, 200 and 250cm\u22121 period modulations also generate frequency component at corresponding frequency as well as its multiple frequency e.g. 150cm\u22121 also generate peak at 300cm\u22121 . 33 \f1.2. Review on Current Coherent Anti-Stokes Raman Scattering Methods phase shaping was applied on the excitation part of single broadband pulse. The excitation part position is shown in \ufb01gure 1.12 for single pulse CARS. In the time domain, the shaped pulse splits into a pulse train. If the pulse train matches the period of a vibrational resonance, it can e\ufb00ectively excite it. In the frequency domain, the self-correlation of such sinusoidal modulated pulse shows maxima at certain frequency and minima at others. This means excitation for certain resonances and suppression for others. A numerical simulation on sinusoidal shaping of a 150fs pulse is presented as \ufb01gure 1.14. The e\ufb00ect of sinusoidal spectral phase modulation in the frequency domain generates modulation on the \ufb01eld correlation of pump and Stokes pulses and achieves the selective excitation. With this scheme, a good resolution pulse shaper can be used to create sinusoidal modulation on a broad band pulse to selectively excite vibration resonances. After the excitation of coherent vibration and probing, the total CARS signal is recorded with respect to the sinusoidal modulation period and is used to generate CARS spectrum. Y. Silerberg and his coworkers [22] further implemented this vibration selection CARS into single beam CARS microscopy. A.G. Motzkus and coworkers [69] further implemented it for low-wavenumber vibration mode (from 50 to 400 cm\u22121 ) spectroscopy. The disadvantage of both chirped approach and sinusoidal modulation approach is still the spectral resolution. In both approaches, the spectral resolution is determined by the excitation selectivity over resonances. Therefore it is limited by the pulse shaping ability. It cannot be better than the SLM pixel bandwidth which is around 10 to 20cm\u22121 . Secondly, both approaches require certain scanning. The chirped pulse approach needs scanning of the time delay and a calibration on the relation between time delay and the excitation frequency for di\ufb00erently chirped pulses. The sinusoidal modulation approach needs to scan the period of sinusoidal phase patterns. The speed of measurement is therefore determined by the pulse shaper response time (The SLM that was used in this thesis work has around a 100ms response time per phase pattern). 34 \f1.2. Review on Current Coherent Anti-Stokes Raman Scattering Methods 1.2.5 Summary and Comparison of Current Methods The narrow band CARS scheme has straightforward spectrum\/resonance interpretations. Due to the long duration of narrow band pulses (from picosecond up to nanosecond), time synchronization between excitation lasers is not a di\ufb03cult problem. With the narrow band probe pulse, the CARS spectrum re\ufb02ects the pro\ufb01le of vibration resonances when the non-resonant background is low. The disadvantage of the narrow band CARS methods is its low signal strength. Narrow band lasers come with lower peak power than that of short pulse duration lasers, and low peak power laser generates low signal in the third order nonlinear optical process of CARS. To obtain detectable signal, laser power has to be set at high level, which could lead to the possible degradation of samples. The narrow band CARS method requires two lasers of di\ufb00erent frequency: typical Nd:YAG laser and a dye laser. It requires frequency tuning of the dye laser, which is time-consuming and susceptible to mechanical instability. The spectral resolution of narrow band CARS is determined by the bandwidth of the excitation pulses, narrow bandwidth leads to high spectral resolution. Multiplex CARS improves the acquisition speed of narrow band CARS by simultaneously accessing multiple resonant levels while maintaining the straight forward spectrum interpretation. It removes the scanning of laser frequencies. The interpretation of the multiplex spectrum is the same as that obtained by narrow band CARS. In terms of experimental setup, the narrow band Nd:YAG laser is used as pump\/probe pulse. A broad band dye laser that is pumped by the narrow band laser provides the broad band Stokes frequency. After the invention of the solid state Ti:sapphire laser, narrow band probe pulses could be created from spectral cutting of broad band pulse[49]. Nonlinear optical parametric process became more e\ufb00ective for high peak power laser pulses, making the frequency conversion convenient. Broad band pulses are used as both pump and Stokes pulse. In both dye laser system and Ti:Sapphire system, the setup of multiplex CARS is based on one source laser, therefore eliminating the \ufb02uctuation that is associated between two laser devices. However, the disadvantage of multiplex CARS 35 \f1.2. Review on Current Coherent Anti-Stokes Raman Scattering Methods is still inherited from the narrow band CARS method: it has low signal strength because of the low peak power of one or two beams. Creating a narrow band probe pulse from broad band femtosecond laser reduces the total signal in multiplex CARS. Moreover, for multiplex CARS methods that involve the usage of narrow band probe cut from broad band radiation, the spectral resolution of CARS spectrum is coupled with the signal intensity. The narrower the probe bandwidth is, the better the spectral resolution, but the lower the signal strength (see \ufb01gure 1.9). The above situation describes a \u201cresolution vs. intensity\u201d dilemma of achieving good spectral resolution versus obtaining high signal strength. A similar and simple example of this dilemma is given by the slit choice of a spectrometer: narrow slits give high resolution but low intensity on the detector. In a frequency domain CARS experiment, the spectral resolution is strictly limited by the bandwidth of the probe pulse. For the experiment that the narrow band probe pulse is obtained through cutting of broad band radiation, a probe pulse of small bandwidth gives good spectral resolution, but reduces the signal strength, thus prolonging the required acquisition time. Probing the vibrational coherence with broad band femtosecond pulse, on the other hand, gives strong signal but very poor, if any, spectral resolution. This dilemma is common for multiplex CARS type of methods, including single pulse CARS techniques [21, 23, 63]. Time-resolved CARS methods provide a fresh approach of temporal domain vibrational spectroscopy. They utilize three ultrafast pulses to obtain the time domain beating response of a vibrational coherence, and give high signal strength by using high peak power broad band pulses. The interpretation on the resonant levels is done by the Fourier transform of the temporal beating. The peaks on the Fourier-transformed have better spectral resolution than the bandwidth of probe pulse. For a Fourier method, the spectral resolution of time-resolved CARS is limited by the duration of time scan, rather than the bandwidth of the probe pulse. However, there is one signi\ufb01cant di\ufb00erence between time-resolved CARS and frequency domain methods. The vibrational beatings retrieved from Fourier analysis is the autocorrelation of the spectrum rather than the spectrum itself (see \ufb01g36 \f1.3. Theory of Coherent Anti-Stokes Raman Scattering ure 1.10). In addition, autocorrelation of a spectrum gives a poor indication of the linewidth of resonances comparing to the spectrum itself, because the line width of peaks are convolved to give the width of the autocorrelation peak in the autocorrelation spectrum. The comparison between \ufb01gure 1.10A and \ufb01gure 1.10D shows this broadening e\ufb00ect. Combination of femtosecond laser sources with pulse shaping techniques open a door to a group of creative CARS methods. The manipulation of a broad band laser \ufb01eld by pulse shaping can assign certain functions to frequency components or lead to possible interference in multi-photon processes. Single pulse CARS greatly simpli\ufb01ed the experimental setup, simplifying the total instruments to perform CARS measurement to an oscillator and a pulse shaper. With pulse shaping, selective excitation is feasible without tuning laser frequencies. However, the spectral resolution of pulse shaping CARS methods is limited by the resolution of the pulse shaper, and the acquisition time is often limited by the response time of the pulse shaper as well. The above discussion provides readers a broad pro\ufb01le of the CARS research. To gain a further insight into the CARS process, a theoretical analysis is necessary and will be presented in the next section. 1.3 Theory of Coherent Anti-Stokes Raman Scattering The purpose of spectroscopy in general is to exploit light-matter interactions to reveal the energy level structure of atoms or molecules. The matter interacts with light \ufb01elds and this interaction a\ufb00ects the properties of light \ufb01elds, whether it is intensity gaining, propagation direction altering or the creation of new frequencies. By measuring the optical \ufb01elds that take part in the interaction, researchers can deduce structural information of the sample. When this general spectroscopy model comes to the speci\ufb01c case of coherent anti-Stokes Raman scattering (CARS), two questions are immediately raised: how does the resonance structure a\ufb00ect the generation of 37 \f1.3. Theory of Coherent Anti-Stokes Raman Scattering the CARS \ufb01eld? and how are spectra of the anti-Stokes \ufb01eld interpreted to give information on resonance structure of samples? Equation (1.1) provides a general formula for CARS signal generation. In this section, detailed analytical discussions on CARS are presented. 1.3.1 Brief introduction to Density Matrix CARS can be treated as a special case of the resonant four-wave-mixing process, therefore it is traditionally described by deriving phenomenological third order susceptibility \u03c7(3) [70, 71]. However, the line width measured by CARS re\ufb02ects a decoherence process between coherently excited levels, comparing to linewidth of Raman spectroscopy that re\ufb02ects the relaxation of population. The treatment of density matrix[71, 72] is particularly convenient in describing coherence between laser excited levels and its time evolutions. The interaction between matter and light is often described by the timedependent Schro\u0308dinger equation: ih\u0304 \u2202\u03c8s (r, t) \u0004 s (r, t) = H\u03c8 \u2202t (1.6) \u0004 can be assumed as summation of Hamiltonian of a molecule H \u00040 Where H and interaction Hamiltonian between external optical \ufb01eld and matter V\u0004 (t) \u0004 =H \u0004 0 + V\u0004 (t) H (1.7) \u0004 0 gives a complete set of basis functions The solution of H \u03c8(t, x) = \u0002 Cn (t)\u03c6n (x) (1.8) n The expansion coe\ufb03cient Cn (t) gives the probability amplitude of the molecule in energy states n and at time t, and the time evolution of the molecule can be described by the evolution of the expansion coe\ufb03cients Cn (t). The real system in experiment consists of many molecules, even in the small interaction region of a tightly focused laser beam, the amount of 38 \f1.3. Theory of Coherent Anti-Stokes Raman Scattering molecules (often > 106 ) is beyond the computational power to track individually. Moreover, there are often collisions happening among molecules, which modify the actual state of involved molecules. In this situation, the density matrix can be used to conveniently describe the ensemble of molecules in a statistical fashion. The elements of the density matrix are de\ufb01ned by \u2217 (t)C (t) \u03c1nm (t) = Cm n (1.9) Where the overbar denotes an ensemble average of all molecules. Subscripts n and m represent the energy levels n and m. The density matrix represents an average of coe\ufb03cient product over all molecules. The diagonal elements of the density matrix \u03c1nn represents the population of molecules in the state n, and the o\ufb00-diagonal elements \u03c1nm represent the coherence between states n and m. They are non-zero when the system is in a coherent superposition of energy eigenstates and zero when system is in thermal equilibrium. This can be created by coherent laser radiations but not through population redistribution through temperature changes. In the density matrix formalism, the expectation value of an observable A is given by the trace of the product between operator matrix A\u0302 and the density matrix \u03c1\u0302 < A >= tr(\u03c1\u0302A\u0302) (1.10) The time evolution of the density matrix follows [71] \u2212i d\u03c1nm = [H\u0302, \u03c1\u0302]nm dt h\u0304 (1.11) which is known as Liouville equation, which is derived from time dependent Schro\u0308dinger equation. Due to collisions or other interactions that drive the system towards thermal equilibrium, there are relaxation terms in both diagonal (population) and o\ufb00-diagonal (coherence)terms of the density matrix. The Liouville equation is then modi\ufb01ed by adding the statistical damping factor \u03b3nm d\u03c1nm \u2212i = [H\u0302, \u03c1\u0302]nm \u2212 \u03b3nm (\u03c1nm \u2212 \u03c1eq nm ) dt h\u0304 (1.12) 39 \f1.3. Theory of Coherent Anti-Stokes Raman Scattering Since in thermal equilibrium, the phase of individual molecules in a given energy level is random, the statistical o\ufb00 diagonal density matrix element \u03c1eq nm is assumed to be zero due to the cancelation of summation over wavefunctions of large number of molecules. The damping factor \u03b3nm re\ufb02ects the rate of relaxation from a coherent superposition of di\ufb00erent states to thermal equilibrium and \u03b3nm = \u03b3mn . Using expression (1.7), the commutator can be separated as [H\u0302, \u03c1\u0302] = [H\u03020 , \u03c1\u0302] + [V\u0302 , \u03c1\u0302] and equation (1.12) can then be expressed as i d\u03c1nm = \u2212i\u03c9nm \u03c1nm \u2212 [V\u0302 , \u03c1\u0302]nm \u2212 \u03b3nm (\u03c1nm \u2212 \u03c1eq nm ) dt h\u0304 (1.13) where \u03c9nm is the energy di\ufb00erence between level n and m, which comes from the stationary Hamiltonian H\u03020 . Equation 1.13 is used as the fundamental equation to describe the behavior of an ensemble of molecules. 1.3.2 CARS Expression Derivation Using Density Matrix Formalism CARS generates a directional coherent signal at the anti-Stokes frequencies. The light emission process is associated with Maxwell\u2019s equations with a source polarization term P\u0005 . \u0005+ \u2212 \u22072 E 1 \u22022 \u0005 4\u03c0 \u2202 2 P\u0005 E = \u2212 c2 \u2202t2 c2 \u2202t2 (1.14) The P\u0005 derives from the macroscopic \u201cpolarization\u201d of the sample [72], which is directly related to the dipole operator \u03bc\u0302, by P\u0005 = N < \u03bc >, where N is the particle number. Taking a two level system as an example, the dipole operator \u03bc\u0302 has the form of \u0006 \u03bc\u0302 = 0 \u03bc12 \u03bc21 0 \u0007 (1.15) note that \u03bc21 = \u03bc\u221712 The expectation value of \u03bc\u0302 is given by expression (1.10). For example if the density matrix of the two level system has the form of 40 \f1.3. Theory of Coherent Anti-Stokes Raman Scattering \u0006 \u03c111 \u03c112 \u0007 \u03c121 \u03c122 , the expectation value of \u03bc is then obtained by the trace of \u03c1\u0302\u03bc\u0302. \u0006 \u03c1\u0302\u03bc\u0302 = 0 \u03bc12 \u03bc21 0 \u0007\u0006 \u03c111 \u03c112 \u0007 (1.16) \u03c121 \u03c122 < \u03bc >= \u03c112 \u03bc21 + \u03c121 \u03bc12 (1.17) Even though expression (1.17) represents the situation of a two level system, for multilevel system, the expectation value of the dipole moment has similar form. Thus the macroscopic polarization P\u0005 depends on the o\ufb00-diagonal elements of the density matrix \u03c1nm . Therefore, the following discussion on CARS in this thesis is based on deriving o\ufb00-diagonal elements of the density matrix resulting from light-matter interaction. The interaction between matter and light is described by equation (1.13). The energy diagram of CARS is shown in \ufb01gure 1.15 It contains three resonant levels, the ground state, vibrational state and an intermediate state at much higher energy. Its density matrix can be represented by a 3 \u00d7 3 matrix spanning the ground state g, vibrational state v and intermediate state i as \ufb01gure 1.15 shows.\u23a1 To simplify the\u23a4discussion, \u03c1eq 0 0 \u23a2 gg \u23a5 eq eq \u23a2 the initial state can be assumed to be \u03c10 = \u23a3 0 \u03c1vv 0 \u23a5 \u23a6. \u03c1vv and \u03c1eq ii \u00051 for Ev \u0006 kb T , and \u03c1eq gg 0 0 \u03c1eq ii \u2248 1 which represents the assumption that majority of molecules are in the ground state in thermal equilibrium. O\ufb00diagonal elements of the matrix are also zero, from the assumption of thermal equilibrium. When interacting with one pulse, o\ufb00-diagonal elements of \u03c1 are prepared, which can be obtained by solving equation 1.13. With initial condition of \u03c10 , and using the perturbation method [71] (assuming \u03c1\u0302 = \u03c1\u0302(0) + \u03c1\u0302(1) + \u03c1\u0302(2) ....), the linear response term of \u03c1\u0302 follows \u2212(i\u03c9nm +\u03b3nm )t \u03c1(1) nm (t) = e \u0003 t \u2212i \u221e h\u0304 \u0002 [V\u0302 , \u03c10 ]nm e(i\u03c9nm +\u03b3nm )t dt\u0004 (1.18) 41 \f1.3. Theory of Coherent Anti-Stokes Raman Scattering Figure 1.15: The energy diagram of CARS, g v and i are three levels involved in derivation. The intermediate electronic level |i >is far from resonance with detuning of \u0394 and \u0394\u0004 42 \f1.3. Theory of Coherent Anti-Stokes Raman Scattering n, m are dummy indices and V\u0302 (t\u0004 ) is the interaction Hamiltonian, which has the form \u23a1 0 \u23a2 \u03bcgv E(t) \u03bcgi E(t) V\u0302 = \u2212 \u23a2 \u23a3 \u03bcvg E(t) 0 \u03bcig E(t) \u03bciv E(t) \u23a4 \u23a5 \u03bcvi E(t) \u23a5 \u23a6 (1.19) 0 Where \u03bcgv is the dipole moment between state g and v, and \u03bcgv = \u03bc\u2217vg . When interaction involves two pulses, as is the case in the vibration preparation step of CARS, the second order expansion of the density matrix \u03c1\u0302(2) is used to re\ufb02ect such preparation. It can be derived as \u0003 t \u2212i \u2212(i\u03c9nm +\u03b3nm )t \u03c1(2) nm (t) = e \u221e h\u0304 \u0002 [V\u0302 , \u03c1\u0302(1) ]nm e(i\u03c9nm +\u03b3nm )t dt\u0004 (1.20) The E \ufb01eld in the interaction Hamiltonian V\u0302 contains the incident pulses. When multiple \ufb01elds exist for excitation, E(t) can take the general form of E(t) = \u0002\u0003 \u221e 0 n En (\u03c9)e\u2212i\u03c9t d\u03c9 + c.c. (1.21) This expression contains both positive frequency and negative frequency components, in order to let the electric \ufb01eld in the time domain be real, since it is a measurable observable. To follow the convention of CARS, in the following derivation we use Ep (t) to describe the \ufb01rst optical \ufb01eld (pump) that interacts with the system, Es (t) to describe the second optical \ufb01eld (Stokes), and Epr (t) to describe the third optical \ufb01eld (probe). The solution of o\ufb00 diagonal elements of \u03c1\u0302(1) in equation (1.20) can be found as (1) \u03c1ig \u22121 = h\u0304 \u03bcig (\u03c1eq gg \u2212 \u03c1eq ii ) (1) eq = h\u0304\u22121 \u03bcvg (\u03c1eq \u03c1vg gg \u2212\u03c1vv ) (1) \u0003 \u221e 0 \u0003 \u221e eq \u03c1vi = h\u0304\u22121 \u03bcvi (\u03c1eq ii \u2212 \u03c1vv ) 0 [ \u0003 \u221e 0 Ep\u2217 (\u03c9)ei\u03c9t Ep (\u03c9)e\u2212i\u03c9t [ + ]d\u03c9 (1.22) (\u03c9ig \u2212 \u03c9) \u2212 i\u03b3ig (\u03c9ig + \u03c9) \u2212 i\u03b3ig Ep\u2217 (\u03c9)ei\u03c9t Ep (\u03c9)e\u2212i\u03c9t + ]d\u03c9 (1.23) (\u03c9vg \u2212 \u03c9) \u2212 i\u03b3vg (\u03c9vg + \u03c9) \u2212 i\u03b3vg [ Ep\u2217 (\u03c9)ei\u03c9t Ep (\u03c9)e\u2212i\u03c9t + ]d\u03c9 (1.24) (\u03c9vi \u2212 \u03c9) \u2212 i\u03b3vi (\u03c9vi + \u03c9) \u2212 i\u03b3vi 43 \f1.3. Theory of Coherent Anti-Stokes Raman Scattering (1) Noted these \ufb01rst order elements \u03c1nm are very small in the situation of CARS, since the excitation \ufb01elds are far from being resonant with either the vibrational state \u03c9gv or intermediate state \u03c9gi . In terms of actual value, (1) (1) (1) \u03c1gi and \u03c1gv \u0006\u03c1vi , because of initial equilibrium diagonal density matrix (1) (1) element of state i being zero. The actual value of \u03c1gi and \u03c1gv depends on the magnitude of detuning \u0394 and \u0394\u0004 . With these expression of \ufb01rst order perturbation solution of density matrix, we continue to check the second order density matrix \u03c1\u0302(2) . The density element corresponding to the coherence between the ground state and the (2) vibrational state, \u03c1vg can be found by solving equation (1.20) as \u03c1(2) vg eq (\u03c1eq ii \u2212 \u03c1vv )\u03bcvi \u03bcig = { h\u03042 \u0002 \u0003 \u221e\u0003 \u221e Ep (\u03c9)Es (\u03c9 \u0004 )e\u2212i(\u03c9+\u03c9 )t d\u03c9 \u0004 d\u03c9 [(\u03c9vg \u2212 \u03c9 \u2212 \u03c9 \u0004 ) \u2212 i\u03b3vg ][(\u03c9vi \u2212 \u03c9) \u2212 i\u03b3vi ] 0 0 + + \u0003 \u221e\u0003 \u221e 0 0 0 Ep (\u03c9)Es\u2217 (\u03c9 \u0004 )e\u2212i(\u03c9\u2212\u03c9 )t d\u03c9 \u0004 d\u03c9 [(\u03c9vg \u2212 \u03c9 + \u03c9 \u0004 ) \u2212 i\u03b3vg ][(\u03c9vi \u2212 \u03c9) \u2212 i\u03b3vi ] \u0003 \u221e\u0003 \u221e 0 \u0002 Ep\u2217 (\u03c9)Es (\u03c9 \u0004 )ei(\u03c9\u2212\u03c9 )t d\u03c9 \u0004 d\u03c9 [(\u03c9vg + \u03c9 \u2212 \u03c9 \u0004 ) \u2212 i\u03b3vg ][(\u03c9vi + \u03c9) \u2212 i\u03b3vi ] \u0003 \u221e\u0003 \u221e \u0002 \u0002 Ep\u2217 (\u03c9)Es\u2217 (\u03c9 \u0004 )ei(\u03c9+\u03c9 )t + d\u03c9 \u0004 d\u03c9} [(\u03c9vg + \u03c9 + \u03c9 \u0004 ) \u2212 i\u03b3vg ][(\u03c9vi + \u03c9) \u2212 i\u03b3vi ] 0 0 eq (\u03c1eq gg \u2212 \u03c1ii )\u03bcig \u03bcvi { \u2212 h\u03042 \u0002 \u0003 \u221e\u0003 \u221e Ep (\u03c9)Es (\u03c9 \u0004 )e\u2212i(\u03c9+\u03c9 )t d\u03c9 \u0004 d\u03c9 [(\u03c9vg \u2212 \u03c9 \u2212 \u03c9 \u0004 ) \u2212 i\u03b3vg ][(\u03c9ig \u2212 \u03c9) \u2212 i\u03b3ig ] 0 0 + + + \u0003 \u221e\u0003 \u221e 0 0 0 Ep\u2217 (\u03c9)Es (\u03c9 \u0004 )ei(\u03c9\u2212\u03c9 )t d\u03c9 \u0004 d\u03c9 [(\u03c9vg + \u03c9 \u2212 \u03c9 \u0004 ) \u2212 i\u03b3vg ][(\u03c9ig + \u03c9) \u2212 i\u03b3ig ] \u0003 \u221e\u0003 \u221e 0 \u0003 \u221e\u0003 \u221e 0 \u0002 Ep (\u03c9)Es\u2217 (\u03c9 \u0004 )e\u2212i(\u03c9\u2212\u03c9 )t d\u03c9 \u0004 d\u03c9 [(\u03c9vg \u2212 \u03c9 + \u03c9 \u0004 ) \u2212 i\u03b3vg ][(\u03c9ig \u2212 \u03c9) \u2212 i\u03b3ig ] 0 \u0002 \u0002 Ep\u2217 (\u03c9)Es\u2217 (\u03c9 \u0004 )ei(\u03c9+\u03c9 )t d\u03c9 \u0004 d\u03c9} [(\u03c9vg + \u03c9 + \u03c9 \u0004 ) \u2212 i\u03b3vg ][(\u03c9ig + \u03c9) \u2212 i\u03b3ig ] (1.25) 44 \f1.3. Theory of Coherent Anti-Stokes Raman Scattering (2) Expression (1.25) is the complete term of vibrational coherence \u03c1gv . Ac(1) (1) (2) cording to equation (1.20), only \u03c1gi and \u03c1iv enters into \u03c1vg . Still, it has a very complex form. It has to be simpli\ufb01ed before being used. Such simpli\ufb01cation can be done by analyzing the major contributions. The resonance \u03c9gv for a typical Raman active sample is from 200cm\u22121 to 4000 cm\u22121 , the intermediate state normally is an electronic state, which varies depending on speci\ufb01c sample, a typical estimation is \u03c9ig > 20000cm\u22121 . The initial equilibrium state \u03c1(eq) can also help simpli\ufb01cation. \u03c1eq ii can be considered as (eq) (eq) zero at equilibrium distribution and \u03c1vv \u0005 \u03c1gg which can be estimated by Boltzmann distribution. With those conditions, one can \ufb01nd that the main resonant term of contribution to CARS process is \u03c1(2) vg (t) = \u2212 \u0003 \u03c1eq gg \u03bcig \u03bcvi h\u03042 \u221e\u0003 \u221e 0 0 \u0002 Ep (\u03c9)Es\u2217 (\u03c9 \u0004 )e\u2212i(\u03c9\u2212\u03c9 )t d\u03c9 \u0004 d\u03c9 [(\u03c9vg \u2212 \u03c9 + \u03c9 \u0004 ) \u2212 i\u03b3vg ][(\u03c9ig \u2212 \u03c9) \u2212 i\u03b3ig ] (1.26) This can be interpreted as a stimulated Raman process, which serves as the \ufb01rst step of CARS excitation (see section 1.1.3). It has the carrier frequency of \u03c9 \u2212 \u03c9 \u0004 . It should be noted that the rest non-resonant terms can (2) create transient coherence of \u03c1vg between the ground state and vibrational state during the pulse excitation, which contributes to the non-resonant background of CARS. It will be discussed in the next section. Expression (1.25) is the general perturbation solution to two-photon process, and expression (1.26) is a specialized expression for stimulated Raman process that is responsible for the vibrational excitation in CARS with considerations of energy levels, equilibrium state population and pump\/Stokes frequencies. Expression (1.26) can be further simpli\ufb01ed by replacing the \u03c9 \u0004 with \u03c9\u2212\u03a9. \u03c1(2) vg (t) = \u2212 \u03c1eq gg \u03bcig \u03bcvi h\u0304 2 \u000e\u221e\u000e\u221e Ep (\u03c9)Es\u2217 (\u03c9 \u2212 \u03a9)e\u2212i\u03a9t d\u03c9d\u03a9 [(\u03c9vg \u2212 \u03a9) \u2212 i\u03b3vg ][(\u03c9ig \u2212 \u03c9) \u2212 i\u03b3ig ] 0 0 (1.27) From expression (1.27), we can de\ufb01ne the response function R(\u03a9) to (2) represent the coherence \u03c1vg in the frequency domain. R(\u03a9) contains the 45 \f1.3. Theory of Coherent Anti-Stokes Raman Scattering pro\ufb01le of the vibrational level (\u03c9vg , \u03b3vg ) and is a result of \ufb01eld excitation strength A(\u03a9) R(\u03a9) \u2261 \u03c1(2) vg (\u03a9) = with Cvg = \u2212 \u03c1eq gg \u03bcig \u03bcvi h\u03042 Cvg \u00b7 A(\u03a9) [(\u03c9vg \u2212 \u03a9) \u2212 i\u03b3vg ] (1.28) which re\ufb02ects the dipole transition strength, and A(\u03a9) = \u0003 \u221e Ep (\u03c9)Es\u2217 (\u03c9 \u2212 \u03a9) 0 (\u03c9ig \u2212 \u03c9) \u2212 i\u03b3ig d\u03c9 (1.29) which re\ufb02ects the preparation power of pump and Stokes pulses. In typical CARS experiment, the pump \ufb01eld is often far o\ufb00 resonant from the intermediate electronic resonant level with detuning \u0394 = \u03c9ig \u2212 \u03c9p \u223c 104 cm\u22121 ), therefore, the denominator term of 1 \u03c9ig \u2212\u03c9\u2212i\u03b3ig in equation (1.29) can be treated as non-resonant excitation therefore be replaced by a real number 1\/\u0394 and can be grouped into Cvg which is now \u2212 \u03c1eq gg \u03bcig \u03bcvi . h\u03042 \u0394 Therefore equa- tion (1.29) can be simpli\ufb01ed as A(\u03a9) = \u0003 \u221e 0 Ep (\u03c9)Es\u2217 (\u03c9 \u2212 \u03a9)d\u03c9 (1.30) Note that in some experiments [14, 73], the pump pulse can be resonant with low electronic states, which will increase the preparation e\ufb03ciency through the resonant denominator. The vibration coherence response function R(\u03a9) prepared by pump and Stokes pulses re\ufb02ects the resonance information of the vibrational level. Figure 1.16 shows the numerical plot of R(t) and R(\u03a9) for a single resonant level (MATLAB simulation script can be found in Appendix A). The resonance is centered at 1000 cm\u22121 and has a FWHM of 12cm\u22121 . The real part of R(\u03a9) \ufb01gure 1.16A shows dispersive pro\ufb01le. The imaginary part shows the Lorentzian pro\ufb01le. Figure 1.16C is the spectrum and spectral phase representation, it is equivalent to the real and imaginary representation shown on \ufb01gure 1.16A and \ufb01gure 1.16B. The spectral phase of R(\u03a9) shows a characteristic \u03c0 radian spectral phase shift across resonance according to expression (1.28). Figure 1.16D shows the time domain R(t) (carrier phase factor ei\u03c9vg t is not shown on this plot). Its amplitude remains zero before the laser pulses 46 \f1.3. Theory of Coherent Anti-Stokes Raman Scattering 0.2 0.3 Amplitude (AU) 0 -0.1 900 950 1000 1050 (B) 0.2 0.1 0 1100 950 Wave number (cm-1) 3 2 1 1050 1100 4 (D) 3 Amplitude (AU) (C) Spectral phase (rad.) Intensity (AU) 4 1000 Wave number (cm-1) 3 2 2 1 Phase (rad.) Amplitude (AU) (A) 0.1 1 0 0 900 0 950 1000 1050 Wave number (cm-1) 1100 -0.5 0 0.5 1 1.5 2 Time (ps) Figure 1.16: This plot is the numerical simulation of one resonant level at 1000cm\u22121 with \u0393 of 6 cm\u22121 . Plot (A) is the real part of R(\u03a9). Plot (B) is the imaginary part of R(\u03a9), which has perfect Lorentzian pro\ufb01le. Plot (C) is R(\u03a9) (solid line) and spectral phase (dashed line) representation of R(t). Plot (D) is the time domain R(t) with intensity (solid line) and phase (dashed line). Carrier frequency is not shown here. 47 \f1.3. Theory of Coherent Anti-Stokes Raman Scattering and free decay after excitation re\ufb02ecting the decoherence coe\ufb03cient \u03b3vg . For femtosecond lasers, their broad bandwidth is capable of simultaneously exciting multiple vibrational states vj . The individual vibrational coherence that broad laser pulses prepare works collectively in coherent antiStokes Raman scattering. The expression(1.28) for the vibrational coherence between the ground state and one vibrational excited state vj can be expanded to expression(1.31) that considers multiple vibrational states covered (2) by the excitation bandwidth. It is a summation of resonant part of \u03c1vi g R(\u03a9) = A(\u03a9) \u0002 j Cj [(\u03c9j \u2212 \u03a9) \u2212 i\u03b3j ] (1.31) This expression shows that the vibrational coherence response function R(\u03a9) has the form of the spontaneous Raman spectra. Its time domain response R(t) can be obtained through straightforward Fourier transform. In chapter 4, an approach of complete characterization of vibrational coherence will be presented that can measure R(\u03a9) of laser induced coherent vibrations. Generation of Coherent Anti-Stokes Field (2) After the preparation of the vibrational coherence \u03c1vg through stimulated Raman, the probe pulse then interacts with the prepared vibrational system to generate signal radiation at the anti-Stokes frequency. From a spectroscopy perspective, the probe pulse measures the prepared system and generates CARS signal carrying the information about the vibrational coherence. In frequency resolved CARS experiments, the bandwidth of the probe pulse is very narrow, thus CARS spectra share the same pro\ufb01le as the vibrational coherence response function R(\u03a9). The only di\ufb00erence between them is the CARS spectrum measured is an array of real values, whereas R(\u03a9) is a complex quantity. Nevertheless, resonant positions and linewidths can be deduced from CARS spectra. However, when the probe pulse has a broad bandwidth, the resemblance between the CARS spectrum and the vibrational coherence is lost. Additional treatments of \ufb01tting are often needed 48 \f1.3. Theory of Coherent Anti-Stokes Raman Scattering to extract resonance positions from the CARS spectrum. In this section, the generation of CARS signal from vibrational coherence will be discussed. The interaction of the probe pulse and the vibrational coherence can also be treated perturbatively, through equation \u2212(i\u03c9nm +\u03b3nm )t \u03c1(3) nm (t) = e \u0003 t \u2212i \u221e h\u0304 \u0002 [V\u0302 , \u03c1(2) ]nm e(i\u03c9nm +\u03b3nm )t dt\u0004 (1.32) (3) Full expansion of \u03c1nm can be really complex. In a similar treatment of \ufb01nding the main resonant term in deriving equation (1.27), equation (1.32) can be solved as (3) \u03c1ig (t) i = e\u2212i(\u03c9ig +\u03b3ig )t h\u0304 \u0003 t \u0002 \u2212\u221e \u0004 i(\u03c9ig +\u03b3ig )t \u03bciv \u03c1(2) dt\u0004 vg Epr (t )e One can replace the probe pulse \ufb01eld with Epr (t\u0004 ) = (2) \u000e\u221e 0 (1.33) Epr (\u03c9 \u0004\u0004 )e\u2212i\u03c9 \u0002\u0002 t\u0002 d\u03c9 \u0004\u0004 + c.c. and \u03c1gv with previous derived expression (1.27), and de\ufb01nition of R(\u03a9), (3) \u03c1ig (t) = 1 h\u0304 \u0002\u0002 \u0003 \u221e\u0003 \u221e R(\u03a9)(\u03c9 \u0004\u0004 )e\u2212i(\u03c9 +\u03a9)t 0 \u03c9ig \u2212 \u03a9 \u2212 \u03c9 \u0004\u0004 \u2212 i\u03b3ig 0 d\u03c9 \u0004\u0004 d\u03a9 (1.34) In terms of excitation frequency, the probe pulse generally is not chosen to be resonant with electronic intermediate state. The detuning \u0394\u0004 = \u03c9ig \u2212 \u03a9 \u2212 \u03c9 \u0004\u0004 is much larger than the damping term \u03b3ig . The factor 1\/(\u03c9ig \u2212 \u03a9 \u2212 \u03c9 \u0004\u0004 \u2212 i\u03b3ig ) can be treated as non-resonant as well, replacing it by 1\/\u0394\u0004 . With this approximation, equation (1.34) can be re-arranged into an explicit form in the time domain (3) \u0004 R(t)Epr (t) \u03c1ig (t) = CR \u0004 = 1\/(h\u0304\u0394\u0004 ) and R(t) = with CR domain, (3) \u03c1ig (t) \u000e\u221e 0 (1.35) R(\u03a9)e\u2212i\u03a9t d\u03a9. It is clear that in the time is a product of vibrational coherence R(t) and probe \ufb01eld Epr (t) CARS signal is generated through the third order polarization P\u0005 (3) , which can be found by extending expression of laser induced dipole moment 49 \f1.3. Theory of Coherent Anti-Stokes Raman Scattering expression (1.17) to the 3 \u00d7 3 density matrix of our three level systems, where the main contribution terms can be found as (3) (3) < \u03bc >= \u03bcgi \u03c1ig + \u03bcig \u03c1gi (1.36) These two terms oscillates at anti-Stokes frequency and corresponds to CARS process, there exist others contribution that are responsible for other FWM frequencies. The generated \ufb01eld Eas is linearly proportional to the third order polarization P\u0005 (3) and P\u0005 (3) = N < \u03bc >, where N is the particle number. Therefore the detectable anti-Stokes signal has the form of \u0004 R(t)Epr (t) + c.c. Eas (t) \u221d CR (1.37) \u0004 . with CR = \u03bcgi CR By the convolution theorem, in the frequency domain, the anti-Stokes \ufb01eld is a straightforward convolution relation between R(\u03a9) and the probe \ufb01eld Epr (\u03c9) in the frequency domain. Eas (\u03c9) \u221d \u0003 \u221e 0 Epr (\u03c9 \u2212 \u03a9)R(\u03a9)d\u03a9 (1.38) It should be noted that both expressions (1.38) and (1.37) assume that the probe pulse does not link the vibrational state v with the intermediate state i. Otherwise, the exact form of expression (1.34) has to be used to describe the process. As a rule of thumb, if the frequency component of the probe pulse is resonant with the energy di\ufb00erence between vibrational states and electronic states \u03c9iv , there will be additional peaks in the CARS spectrum. The possibility of preparing multiple resonant levels with broad band pulses is considered through R(\u03a9) in equation (1.31). As a summary, we \ufb01nd that the probing step of CARS is quite simple and straight forward. In the time domain, the CARS signal is the multiplication between the vibrational coherence R(t) and the probe pulse. In the frequency domain, it is a convolution between the vibrational coherence 50 \f1.3. Theory of Coherent Anti-Stokes Raman Scattering Pump and Stokes Pulses Resonant level information Vibrational coherence Probe pulse CARS signal Figure 1.17: The pink arrows show the information \ufb02ow along physical interactions, and the green dashed arrow shows the information \ufb02ow of data processing. Pump and Stokes pulses prepare vibrational coherence based on the information of molecular resonant levels. Vibrational coherence contains the information of excitation and resonances. Then, vibrational coherence scatters probe pulse to give detectable CARS signal. The shape of CARS signal is determined by the vibrational coherence and the probe \ufb01eld. The task for spectroscopist is to analyze the CARS spectrum to deduce the vibration resonant structure of molecule in data analysis, where the information \ufb02ow is from CARS spectrum back to vibrational resonances. 51 \f1.3. Theory of Coherent Anti-Stokes Raman Scattering and the probe pulse. From the information point of view, the scattering of the probe pulse can be treated as a transfer of information from the not directly measurable vibrational coherence R(\u03a9) to the directly measurable CARS spectrum by frequency convolution. This is a rather general approach in spectroscopy. Considering the fact that the vibrational coherence R(\u03a9) contains the structural information of vibrational resonances, the tasks of CARS spectroscopy are \ufb01rst to prepare vibrational coherence R(\u03a9) and then to probe R(\u03a9) to reveal the pro\ufb01le of vibrational resonances. Figure 1.17 depict such relations. 1.3.3 Non-resonant Background For a spectroscopic method, the measured signal should re\ufb02ect and preferably only re\ufb02ect the energy levels of the sample. Photons that are of same frequency as the signal but come from processes that do not involve energy levels of the sample are detrimental to the measurement. A case in point is the \ufb02uorescence background of spontaneous Raman spectroscopy that covers the Stokes region of the spectrum. CARS methods do not su\ufb00er from \ufb02uorescence background as spontaneous Raman does, because the anti-Stokes signal is blue-shifted from the frequency of the probe pulse which most \ufb02uorescence is red-shifted from the incident light \ufb01eld. But CARS does su\ufb00er from a non-resonant background, which comes from the non-resonant other four-wave-mixing pathways that gives the same frequency photons as the CARS signal that re\ufb02ects vibrational levels. Figure 1.18 shows the optical pathway of some possible FWM processes that lead to a non-resonant response of anti-Stokes frequency under the interaction of broad band pump, Stokes and probe pulses. The theoretical interpretation of non-resonant background can be found as the transient coherence that is prepared during laser pulses interaction with sample when all three pulses temporally overlap. More precisely, it is (3) the summation of the non-resonant terms of \u03c1ig that does not evolve through the resonant state |v >. The source of non-resonant background can be separated into two categories: the \ufb01rst one comes from the transient coherence 52 \fFWM Pump Stokes Probe Stokes FWM Pump Probe FWM Pump Probe Stokes 1.3. Theory of Coherent Anti-Stokes Raman Scattering (v) (g) (A) (B) (C) Figure 1.18: Path (A) and (B) are the degenerate pathways that emit photon at CARS signal frequency but do not prepare vibrational coherence. Path (C) is the condition that probe pulse serves as pump pulse and due to their potentially di\ufb00erence in frequency, it does not prepare vibrational coherence in the intended frequency range. All three scenarios can give signal at the anti-Stokes frequency. There are also other pathways that lead to degenerate frequency at anti-Stokes frequency. 53 \f1.3. Theory of Coherent Anti-Stokes Raman Scattering (2) (2) of \u03c1gv and \u03c1vg from the non-resonant terms of equation (1.25). They are (2) (2) part of the vibrational coherence \u03c1gv or \u03c1gv , but does not directly re\ufb02ect the vibrational pro\ufb01le. The second type of non-resonant background comes from other four-wave mixing pathways that prepare transient \u03c1(3) . There is one common behavior of these two sources of non-resonant responses, that is the requirement of all three pulses overlapping in time. Therefore it can be derived from the time \ufb01eld product of pulses. CN R (t) \u221d Ep (t)Es (t)Epr (t) (1.39) where CN R (t) is the time domain response of multiple non-resonant pathways. Note that the time domain optical \ufb01elds are real and contain both positive frequency and negative frequency En (t) = \u000e\u221e 0 E(\u03c9n )e\u2212i\u03c9n t d\u03c9 + c.c.. Thus CN R (t) has multiple terms at di\ufb00erent carrier frequencies, such as \u03c9p + \u03c9s + \u03c9pr or \u03c9p + \u03c9s \u2212 \u03c9pr . The term that has \u03c9p + \u03c9s \u2212 \u03c9pr is of the same frequency as CARS signal, and it leads to the non-resonant background of CARS. Using the convolution theorem and equation (1.30), we can obtain the frequency domain equivalent of equation (1.39) that gives \u03c9p + \u03c9s \u2212 \u03c9pr as EnR (\u03c9) \u221d with A(\u03a9) = \u000e \u0003 A(\u03a9)Epr (\u03c9 \u2212 \u03a9)d\u03a9 (1.40) Ep (\u03c9)Es\u2217 (\u03c9 \u2212 \u03a9)d\u03c9. With these expressions, the overall expression for CARS signal including non-resonant response can be found as follows: \u0002 R( \u03a9) = [ v Cv + CnR ]A(\u03a9) (\u03c9gv \u2212 \u03a9) \u2212 i\u03b3gv ECARS (\u03c9) \u221d \u0003 R(\u03a9)Epr (\u03c9 \u2212 \u03a9)d\u03a9 (1.41) (1.42) Where R(\u03a9) is the adjusted generalized vibrational coherence between vibration excited states and the ground state with non-resonant background (comparing to equation (1.31)). In the discussion of this thesis, R(\u03a9) is assumed to contain the non-resonant background. Hence, the \ufb01nal expressions (1.41) and (1.42) are obtained for CARS. They will serve as basic formulae 54 \f1.3. Theory of Coherent Anti-Stokes Raman Scattering for the following chapters of this thesis. The e\ufb00ect of non-resonant background leads to dispersive pro\ufb01les in CARS spectra. Due to the coherent nature of CARS signal, the background subtraction of CARS spectra cannot be e\ufb00ectively done. In chapter 5, a new approach based on characterization of vibrational coherence R(\u03a9) is introduced to address this problem. 1.3.4 Sample Numerical Simulation This section shows the numerical simulation of broad band CARS using expressions derived in previous section. The simulation starts from a numerical creation of ultrafast pulses as an array of values and coordinates. The original unshaped pulse in the frequency domain is assumed to be Gaussian and transform-limited. as the expression(1.43) shows: Ei (\u03c9) = exp(\u2212 (\u03c9 \u2212 \u03c9ci )2 ) 2W 2 (1.43) with \u03c9ci being the central frequency and W being the width of the pulse spectrum. In terms of data structure, Ei (\u03c9) is stored as an array of complex value corresponding to a coordinate array \u03c9. In the simulation, pump Stokes and probe \ufb01eld arrays are created as Ep (\u03c9), Es (\u03c9) and Epr (\u03c9) respectively. The simulation code for generating a pulse can be found in appendix A.1. The e\ufb00ect of pulse shaping on the created pulse arrays is equivalent to applying spectral phase and amplitude masks at the corresponding coordinate. A pulse shaper array can be created according to expression(1.44), with the same coordinate \u03c9 as the pulse that it works on. M (\u03c9) = M0 (\u03c9)ei\u03c6M (\u03c9) (1.44) It should re\ufb02ect the discrete property of shaper pixels (described in section 1.4). The shaping in the simulation is achieved by multiplying shaping array M (\u03c9) with pulse array Ei (\u03c9). The frequency domain expression after the pulse shaper is: 55 \f1.3. Theory of Coherent Anti-Stokes Raman Scattering Ep (\u03c9) = M (\u03c9) \u00b7 Ei (\u03c9) (1.45) After obtaining the frequency domain pulse array after the pulse shaper, Fourier transform is used to convert it to the time domain array Ep (t) = f f t(Ep (\u03c9)) with corresponding coordinate in time domain t. The step size of the time domain coordinate can be calculated by \u0394t = 1\/(max(\u03c9) \u2212 min(\u03c9)), where max(\u03c9) and min(\u03c9) are the maximal and minimal value of the frequency coordinate. To avoid fast phase oscillations, the carrier frequency is tracked separately. Figure 1.19 shows the numerical plot of ultrafast pulses with and without the sinusoidal spectral phase pulse shaping. The time domain electric \ufb01eld array for pump, Stokes and probe pulses are generated as Ep (t),Es (t) and Epr (t). The simulation code for pulse shaping can be found in appendix A.2. The \ufb01eld product A(t) of pump and Stokes pulses in the time domain is given by expression(1.46) A(t) = Ep (t) \u00b7 Es\u2217 (t) (1.46) A point worth noting is that the Stokes pulse serves as stimulated emission, so the complex conjugate value is used. Such multiplication is done element by element, and the result is an array. The vibrational coherence R(t) is the convolution between the resonance Lorentzian and the \ufb01eld product A(t). The MATLAB[74] is very e\ufb03cient performing discrete Fourier transform and slow on numerical convolutions. To reduce the computational time, the time domain convolution is done in the corresponding frequency domain as multiplication. A(t) is converted to the frequency domain using an inverse Fourier transform A(\u03a9) = \ufb00t\u22121 {A(t)}. Its coordinate array is now \u03a9, centered at the carrier frequency di\ufb00erence of pump and Stokes pulse. The resonances are represented using Lorentzian pro\ufb01le L(\u03a9) by expression(1.47): \u0002 L(\u03a9) = [ i Ci + CnR ] (\u03c9i \u2212 \u03a9) \u2212 i\u03b3i (1.47) 56 \f1.3. Theory of Coherent Anti-Stokes Raman Scattering with \u03c9i and \u03b3i being the resonant level and line width of respective vibrational resonant levels. The coordinate of this array is \u03a9, the same as the \ufb01eld correlation array P (\u03a9), since the range of frequency di\ufb00erence between pump and Stokes pulses should cover those resonances. The vibrational coherence R(\u03a9) is then given by R(\u03a9) = L(\u03a9) \u00b7 P (\u03a9). The Fourier transform of R(\u03a9) gives vibrational coherence in the time domain R(t), which is then multiplied by the time domain probe \ufb01eld Epr (t) to generate CARS signal in time ECARS (t). If the probe pulse has time delay with respect to pump and Stokes pulses, it can be introduced at this step by shifting its envelope within the coordinate array. The CARS spectrum then can be obtained by inverse Fourier transform: ECARS (\u03c9 \u0004 ) = \ufb00t\u22121 {ECARS (t)}. Figures 1.20 A and B show the plot of vibrational coherence in both the frequency and the time domains. We can see that the frequency domain R(\u03a9) re\ufb02ects the resonance pro\ufb01le with clear peaks and line width. The simulation code for CARS generation can be found in appendix A.3. The spectral pro\ufb01le of CARS is dependent on the vibrational coherence ,R(t), and the amplitude and phase shape of the probe pulse, Epr (t). The pro\ufb01le of CARS under broad band excitation of phase shaping may not necessarily re\ufb02ect the energy level pro\ufb01le. Figure 1.20 shows the comparison of CARS spectra between the probe pulse shaping of \u03c0 phase step (blue line \ufb01gure 1.20C) and of sinusoidal phase shaping (red dashed line \ufb01gure 1.20C). They have very di\ufb00erent pro\ufb01les comparing to the spectrum of the vibrational coherence R(\u03a9) that is shown in \ufb01gure 1.20A. Moreover, the spikes in the spectrum do not necessarily correspond to the location of resonances. The CARS spectra with unshaped probe pulse are shown in \ufb01gure 1.20D as reference. It gives poor spectral resolution due to the broad bandwidth and \ufb02at spectral phase of probe pulse. 1.3.5 Phase Matching Consideration CARS signals are coherent. Being coherent has twofold meanings for CARS: \ufb01rstly, CARS photons propagate along a certain \ufb01xed direction. Secondly, 57 \f1.3. Theory of Coherent Anti-Stokes Raman Scattering B 5 Intensity 4 3 2 Phase (rad) A 1 1.2 1.25 1.3 1.35 x 104 -60 -40 -20 0 20 40 60 0 80 3 Intensity 2.5 C 6 D 5 2 4 1.5 3 1 2 0.5 Phase (rad) 1.15 1 0 0 1.15 1.2 1.25 Frequency 1.3 1.35 x 104 (cm-1) -200-150-100-50 0 50 100 150 200 Time (fs) Figure 1.19: (A) is the frequency domain plot of intensity (blue line) of unshaped pulse with 400cm\u22121 bandwidth and spectral phase (dashed red line). (B) is the plot of this unshaped pulse in the time domain. (C) shows the plot of intensity (blue line) and shaped spectral phase (dashed line) by pulse shapers. (D) shows the time domain plot for a shaped pulse. The phase jump at 150fs is because for phase 0 equals to 2\u03c0 . The carrier frequency is not shown in the time domain plot. 58 \f1.3. Theory of Coherent Anti-Stokes Raman Scattering 6 1 A 45 B 40 5 30 25 0.5 3 20 Phase Intensity 35 4 15 2 10 1 5 0 0 600 800 1000 1200 0 0 0.5 1 1.5 2 2.5 Time (ps) Frequency (cm-1) 1 Intensity C D 0.5 0 720 740 760 wavelength (nm) 780 720 740 760 780 wavelength (nm) Figure 1.20: (A) is the frequency domain plot of the vibrational coherence of multiple levels prepared by transform limited pump and Stokes pulses with 400cm\u22121 bandwidth. Intensity is plotted as thick blue line and spectral phase as dashed red line. (B) is the plot of the vibrational coherence in the time domain. Intensity is plotted as blue line and spectral phase as red dashed line. (C) is the CARS spectra generated with \u03c0 phase step probe pulse (blue line) and with sinusoidal spectral phase shaping (red line). (D) shows the CARS spectrum using a transform-limited probe pulse. 59 \f1.3. Theory of Coherent Anti-Stokes Raman Scattering CARS signals generated at di\ufb00erent locations in the sample can constructively or destructively interfere with each other. These two facts bring forward questions on determining the signal direction and avoiding destructive interference of signal. The answer to the \ufb01rst question involves the propagation k vector in space, and the answer to second question leads to the phase matching condition[71] consideration. The typical e\ufb03cient coherent anti-Stokes Raman scattering process satis\ufb01es both the energy conservation expression(1.48) and momentum conservation expression(1.49). \u03c9as + \u03c9s = \u03c9p + \u03c9pr (1.48) k as + k s = k p + k pr (1.49) where k i is the k vector of light \ufb01elds. The momentum conservation expression(1.49) can be used explicitly to estimate the propagation direction of the CARS signal direction. However, the sample has its own dispersion property ki = ni \u03c9i \/c, satisfying expression(1.48) in a condensed phase leads to | k as ks kp k pr |+| |=| |+| | nas ns np npr (1.50) Where ni is the respective refractive index at corresponding frequencies. Both expressions must be satis\ufb01ed in order to e\ufb03ciently generate CARS signal. If all pulses are collinearly propagating through the sample, it requires the refractive indices satisfy nas = ns = npump = nStokes , which is often not true for condensed matter samples. If the refractive index is not constant across those frequencies, there will be a phase mismatch factor de\ufb01ned as \u0394k = np \u03c9p \/c + npr \u03c9pr \/c \u2212 nas \u03c9as \/c \u2212 ns \u03c9s \/c (1.51) This enters the spatial terms of Maxwell\u2019s equation 1.14, and re\ufb02ects the mismatch between the phase di\ufb00erence of the generated CARS \ufb01eld and the propagating CARS signal \ufb01eld. The e\ufb00ect of phase mismatch due to the dis- 60 \f1.3. Theory of Coherent Anti-Stokes Raman Scattering Figure 1.21: (A) shows situation of phase mismatch. The CARS signals generated as di\ufb00erent location of sample along the propagation direction have di\ufb00erent phase (represented by the direction of arrows) and they add coherently. Such phase mismatch leads to destructive interference at certain distance as the amplitude summation vs. accumulation length plot shows. Figure (B) shows the situation with phase mismatch. All CARS signals add constructively, leads to linear increase of signal amplitude vs. accumulation length. 61 \f1.3. Theory of Coherent Anti-Stokes Raman Scattering persion property of sample in the collinear geometry is schematically shown in \ufb01gure 1.21. We can see the phase mismatch \u0394k leads to destructively interference along the signal accumulation direction. Under collinear focusing geometry, one way to battle such destructive interference is to shorten the signal accumulation length by using tight focusing. Tight focusing by high numerical aperture lens reduces the CARS interaction length, therefore avoiding the destructive inference. The phasematching length can be de\ufb01ned as zc = 2\/\u0394k to help the selection of focusing lens. The confocal parameter of lens should be smaller than zc . This tight focus collinear phase-matching scheme has been widely used in single pulse CARS spectroscopy and CARS microscopy. In non-collinear geometry, expression (1.48) and expression (1.49) can be achieved without strict requirement on focusing condition. The BOXCARS [75] geometry is a popular phase matching geometry for CARS spectroscopy. It arranges the position of three excitation pulses in space such that it occupies three corners of a box (as \ufb01gure 1.22B shows) before focusing by a lens or mirror. After focused on the sample, the signal should propagate along the remaining corner of the box. The k vectors of the pump, probe and Stokes pulses are not within the same plane spatially. Under such geometry, there exists a solution for kas such that \u0394k = 0 and signals generated in the interaction region constructively can interfere to give good signal strength. Figure 1.22 shows the spatial arrangement of the beams. Either the tight focusing collinear geometry or BOXCARS geometry can generate good strength CARS signals. Due to the advantage of easier signal separation, BOXCARS geometry was used for proof-of-principle experiments in chapter 2 to chapter 5. The tight focus collinear geometry was used for the single pulse Noise-autocorrelation CARS experiment in chapter 2 and in some microscopy experiments that are not included in this thesis. 62 \f1.4. Experimental Setup and Pulse shaper (B) (A) k Sto es Pro be Pum p Stokes Pump s oke i-St t n A Probe Anti-Stokes Figure 1.22: (A) schematically shows the direction and amplitude of k vector of pump, Stokes and probe photons in BOXCARS geometry and corresponding k vector of anti-Stokes photon. (B) shows the spatial position of pulses after interaction on samples. The pump, Stokes, probe pulse and generated anti-Stokes pulse are approximately at four corners of a rectangle. 1.4 1.4.1 Experimental Setup and Pulse shaper Overview This thesis focuses on developing CARS methods with broadband coherent pulses. The experimental setup of CARS with broad band lasers is di\ufb00erent from that of traditional CARS methods with narrow band lasers. There are two major di\ufb00erences. Firstly, the excitation and probing pulses are broadband pulses which are from solid state Ti:Sapphire lasers and optical parametric ampli\ufb01ers (OPA) rather than Nd:YAG and dye lasers. The second di\ufb00erence is the extensive usage of the pulse shaping technique for the phase and amplitude manipulation of broad band coherent pulses. One typical CARS setup is shown in \ufb01gure 1.23, which consists of a Ti:Sapphire ampli\ufb01er, an optical parametric ampli\ufb01er(OPA) and a home-built pulse shaper. When building an experimental setup for femtosecond CARS with pulse shaping capability, there are four major considerations. Firstly, the choice of light sources, which includes the fundamental laser radiation generation and frequency conversions. Secondly, implementation of pulse shaping on the excitation pulses, which involves the building of pulse shaper devices and calibration of the spatial light modulator (SLM). Thirdly, signal generation, 63 \f1.4. Experimental Setup and Pulse shaper Figure 1.23: This \ufb01gure shows the setup of a typical BOXCARS geometry CARS experiment with a pulse shaper. The fundamental radiation is generated by a regenerative ampli\ufb01er (block 1). The optical parametric ampli\ufb01er provides the new frequencies for CARS (block 2). A pulse shaper modi\ufb01es the amplitude and phase of laser radiation (block 3). The pulses are synchronized by translation stages (block 4) and are focused on the sample in a noncollinear geometry (block 5). Necessary signal \ufb01ltering is implemented to improve the quality of the signal which is detected by a spectrometer with CCD (block 6) and the Labview program on a computer records the signal and controls elements of the experiment. 64 \f1.4. Experimental Setup and Pulse shaper which involves the optical setup and alignment, pulse spatial overlap on the sample and time synchronization. This part varies a lot depending on the actual project. Fourthly, the signal \ufb01ltering and detection, which can involve spatial \ufb01ltering, utilization of polarization and dichroic \ufb01lters. For the selection of fundamental radiation, the properties of the laser systems need to be considered. These are the central frequency of the output, the duration of pulse, the per pulse energy and the repetition rate. The solid state Ti:Sapphire laser can provide laser radiation from 700nm to 900nm. The pulse duration of Ti:Sapphire lasers can be fewer than two optical cycles (<5.3fs) [76] to picosecond range. There are two kinds of Ti:Sapphire lasers available, the Ti:sapphire oscillator and Ti:Sapphire ampli\ufb01er. An oscillator system provides high repetition rate ( 80MHz), low pulse energy ( 10 nJ) laser radiation, while the ampli\ufb01er system provides low repetition rate ( 1kHz), high pulse energy (1 mJ per pulse) laser radiation. Since CARS is a third order nonlinear process, higher peak power gives higher per pulse signal. Even considering the low repetition rate, an ampli\ufb01er system can generate more signal than an oscillator system for the same amount of total pulse energy. To provide a broad band tunable radiation, an optical parametric ampli\ufb01er (OPA) is used. The major advantage of OPA is its easy frequency tunability. It can provide a wide range tunable output (from 300to 2000nm) at good e\ufb03ciency (about 25% of total input). In CARS, the pulses from the ampli\ufb01er and OPA are used as pump, Stokes and probe pulses. The pulse shaping technique can tailor the amplitude and phase pro\ufb01le of the ultrafast pulses to allow sophisticated control over multi-photon processes. When building the pulse shaper, the speci\ufb01cations of optical elements should be considered. The choices of collimating mirrors and gratings are a\ufb00ected by the bandwidth of input laser \ufb01eld and the window width of the spatial light modulator. The spatial light modulator is controlled by the voltage at each pixel. Since the purpose of the pulse shaper is to introduce phase shifts to the light \ufb01eld at di\ufb00erent frequencies, it requires calibration to convert the voltage value of each pixel of the SLM into an optical phase shift. Details on pulse shapers will be discussed in the pulse shaping section. 65 \f1.4. Experimental Setup and Pulse shaper There are two types of CARS experimental setup: BOXCARS geometry setup and single pulse collinear geometry setup. Figure 1.23 shows the scheme of a typical BOXCARS geometry experiment with a pulse shaper. The optical scheme of a common single pulse CARS experiment is shown in \ufb01gure 1.24. When comparing these two setups, the CARS signal from the BOXCARS geometry is automatically separated from the residual excitation beams, whereas in the collinear geometry the excitation beams have to be \ufb01ltered out from the signal. From the experiment technique consideration, the BOXCARS geometry setup needs beam alignment and pulse synchronization and the single pulse CARS with collinear geometry does not need pulse synchronization at all and is easier to build. The choice between the BOXCARS geometry and single pulse collinear geometry is based on the experiment needs. The CARS signal is detected by a spectrometer with a CCD detector. It is straightforward to set up the detection optics. The important part is to improve the signal to noise ratio by implementing spatial \ufb01ltering, polarization \ufb01ltering as well as usage of dichroic \ufb01lters. 1.4.2 Ti:Sapphire Generative Ampli\ufb01er and OPA Regenerative Ampli\ufb01er A regenerative ampli\ufb01er laser system has the ability to provide high energy (>1mJ), short duration (35 to 150fs) laser pulses. The Spit\ufb01re regenerative Ti:Sapphire ampli\ufb01er system (Spectra Physics) is a commercially available regenerative ampli\ufb01er of 100fs pulse output at 800nm with up to 2w output power (at 1kHz repetition rate). It was used in the \ufb01rst two years of research. The Spectra Physics Spit\ufb01re Pro is the upgraded version of Spit\ufb01re with shorter output duration (40fs) and higher output power of 3w (at 1kHz repetition rate). It was used in the later half of the research in this thesis. Both systems share a similar design and use the chirped pulse ampli\ufb01cation technology [77]. Laser radiation starts as lower energy \u201cseed\u201d pulses from an oscillator at a high repetition rate (80MHz). The peak power of such pulse is below 66 \f1.4. Experimental Setup and Pulse shaper Figure 1.24: This \ufb01gure shows the optical scheme of a collinear geometry single pulse CARS experiment. It has four key parts, the broadband coherent light source (1), a pulse shaper (2), tight focusing and collimating microscope objectives (3) and spectrometer with proper \ufb01lters (4). 67 \f1.4. Experimental Setup and Pulse shaper the damage threshold of the Ti:Sapphire crystal and the mirrors. But the ampli\ufb01ed pulse has high peak power (about 5 orders of magnitude higher peak intensity than the seed pulse) and is capable of damaging the optics. The technique of chirped pulse ampli\ufb01cation is used to tackle this problem. It \ufb01rst utilizes a grating pair to introduce chirp into the seed pulse. Then the chirped seed pulse undergoes ampli\ufb01cation by passing through a Ti:Sapphire crystal multiple times. After ampli\ufb01cation, the ampli\ufb01ed chirped pulse is re-compressed into a short duration high power pulse by a grating pair compressor. By doing so, the high peak power laser \ufb01eld is only present at the output, therefore avoiding damage to the optics during the ampli\ufb01cation. The regenerative ampli\ufb01er utilizes a laser cavity for multiple pass ampli\ufb01cation. The output beam has good beam quality with a diameter of 8mm and pulse energy of 2mJ\/3mJ (Spit\ufb01re\/Spit\ufb01re Pro). The shortest possible output pulse duration of the regenerative ampli\ufb01er is determined by the bandwidth of the output spectrum. The Spit\ufb01re Pro can give around 40fs output duration with 400cm\u22121 FWHM bandwidth. To achieve the shortest possible pulse duration, the grating pair compressor has to be adjusted to compensate the chirp that is introduced by the stretcher grating pair. The distance between the compressor gratings determines the amount of the compensation chirp. In Spit\ufb01re Pro, a motorized translation stage was mounted inside the compressor to adjust the chirp compensation. An auto-correlator (Pulsescout, Spectra Physics) was used to monitor the pulse duration of output pulse. If an auto-correlator is not available, a nonlinear type-I BBO crystal can be used to qualitatively monitor the duration of output pulses by adjusting the compressor to \ufb01nd highest second harmonic generation signal from the crystal. Another e\ufb00ective way of grating distance adjustment is using a short focus lens to focus the output beam into the air. The focused femtosecond laser generates plasma when the pulse has a short duration. The sound of the plasma from Spit\ufb01re Pro is audible at the frequency of 1k Hz. Therefore, the optimal position of compressor gratings can be found with the maximal sound from plasma. Operational tips on simple maintenance are included in the user manual of Spit\ufb01re Pro. Simply put, the mirrors of the regenerative cavity have to 68 \f1.4. Experimental Setup and Pulse shaper be kept clean. The seed beam should be e\ufb03ciently overlapping with cavity optical path of the ampli\ufb01er and diode pump beams at the ampli\ufb01cation crystal. Optical Parametric Ampli\ufb01er A typical CARS experiment in the BOXCARS geometry requires multiple frequencies to serve as separate pump, Stokes and probe pulses. Even though a single pulse CARS experiment uses only one broad band laser, it cannot be applied to high wave number spectroscopy ( 1000cm\u22121 ) because of the bandwidth limitation (a 40fs duration laser pulses has FWHM bandwidth of 400cm\u22121 ). For applications on high wave number spectroscopy, e.g. the C-H stretch at around 3000cm\u22121 , a separate tunable frequency source must be included into the CARS experimental setup. The optical parametric ampli\ufb01er (OPA) is suitable for this task. It can generate radiation from 300nm to 2000nm. The OPA used in our experiment (TOPAS, Light Conversion) gives a total conversion e\ufb03ciency of 20% to 30%, when it is pumped by the regenerative ampli\ufb01er (Spit\ufb01re Pro) at 1 mJ input. The bandwidth of the OPA output is roughly the same as the bandwidth of the input pump beam (400cm\u22121 ). The OPA working mechanism is based on the nonlinear optical process of di\ufb00erent frequency generation (DFG) as shown in \ufb01gure 1.25A. A high intensity pump laser (800nm) is converted into two infrared lasers (signal \u03c9s and idler \u03c9i ) with tunable frequencies. The frequency tunability is done through angle tuning of the nonlinear crystal. The central frequencies of the output beams satisfy the relation of \u03c9f = \u03c9s + \u03c9i with \u03c9f being the pump frequency that comes from Spit\ufb01re Pro. The polarization of the signal beam is the same as the fundamental pump beam (as both are the ordinary polarization to the optical axis of the nonlinear crystal), and the idler polarization is perpendicular to the pump and signal beam (as it is the extraordinary polarization to the axis of the nonlinear crystal). Figure 1.25B shows the schematic of an OPA device. The frequency conversion starts from the generation of continuum white light. A small 69 \f1.4. Experimental Setup and Pulse shaper e B output c b idler pump Signal A d a input Figure 1.25: (A) shows the di\ufb00erence frequency generation that is used in an OPA. (B) shows the schematics of one OPA. The pump beam generates white light at sapphire plate (a), and it is ampli\ufb01ed at an angle-tuned thin BBO nonlinear crystal (b), and \ufb01nally high intensity ampli\ufb01cation is done at a LBO nonlinear crystal (c). The delay lines (d) and (e) are used for the time delay adjustment. 70 \f1.4. Experimental Setup and Pulse shaper fraction of fundamental radiation (4% of fundamental 800nm from Spit\ufb01re Pro) is focused on a sapphire plate to generate uniform and stable white light; then the white light interacts with a fraction of the pump beam intensity (10%) on an angle-tuned BBO (\u03b2-barium borate) nonlinear crystal with good spatial and temporal overlap. The frequency selection is done by tuning the angle of the thin BBO crystal. After the ampli\ufb01cation, the seed beam is collimated and synchronized with remaining high intensity fundamental radiation, and the collimated beams propagate collinearly through a second BBO or a LBO (lithium triborate) nonlinear crystal to give the signal and idler infrared radiations. In CARS experiments, one OPA can be used to provide two frequencies for pump and Stokes pulses. The idler radiation from the OPA is frequency doubled by an additional BBO crystal to give the pump pulse in CARS. Since the polarization of the signal and the idler beams are perpendicular to each other, a BBO crystal is used directly at the output of OPA without using a beam separator. The signal radiation is used as the Stokes pulse in CARS. If the interesting vibrational resonance is at frequency \u03a9, the angle of BBO crystals in OPA should be tuned to provide the signal beam central frequency \u03c9s at (2\u03c9f \u2212 \u03a9)\/3, and the accompanied idler beam \u03c9i at (\u03c9f + \u03a9)\/3. In this condition, the frequency di\ufb00erence between the second harmonic of idler and the signal pulses equals to \u03a9. 1.4.3 Pulse Shaping Techniques Principle The schematic of a common 4-f[20] geometry pulse shaper is shown in \ufb01gure 1.26. Each optical element of the pulse shaper corresponds to a mathematical operation starting with a pulse in time domain E(t). The grating and collimating lens (as \ufb01gure 1.26(A) shows), perform Fourier transform on the time domain pulse E(t) to the frequency domain E(\u03c9) along the Fourier plane. This operation breaks the short duration pulse into long time duration frequency components along the Fourier plane and it is equivalent to \ufb00t[E(t)](\u03c9). A spatial Light Modulator(SLM) is placed in the Fourier plane. 71 \f1.4. Experimental Setup and Pulse shaper A B C Figure 1.26: This \ufb01gure schematically shows the con\ufb01guration of pulse shaper: The optical elements inside box(A) consist of a grating and a collimating lens, their function is to disperse broadband light according to their frequency component. (B) is the liquid crystal based spatial light modulator. It is an array of many independently controllable pixels. The SLM is placed on the Fourier plane of collimating lens, its function is to adjust the amplitude and phase of individual frequency components. Box (C) is the \u201cmirror\u201d setup of (A), its function is to combine beams of di\ufb00erent frequency components into a single pulse. The SLM (\ufb01gure 1.26(B)) modi\ufb01es the amplitude and phase of each frequency component independently through the voltages applied on each SLM pixel. This operation mathematically corresponds to \ufb00t[E(t)](\u03c9)\u00b7A(\u03c9)ei\u03c6(\u03c9) . After amplitude or spectral phase modi\ufb01cation, the collimating element and grating of \ufb01gure 1.26(C) reconstruct the pulse back to a short duration, performing an inverse Fourier transform from the frequency domain back to the time domain. After this operation, the \ufb01nal expression for pulse shaping can be found as: E(t\u0004 ) = i\ufb00t[\ufb00t[E(t)](\u03c9) \u00b7 A(\u03c9)ei\u03c6(\u03c9) ](t) (1.52) with E(t\u0004 ) being the \ufb01eld of the output shaped pulse in the time domain. Its pro\ufb01le is now a function of the amplitude mask, A(\u03c9), and the phase mask, \u03c6(\u03c9), which are adjustable through applied voltages on SLM pixels. A point worth noting is the pixelization of the light \ufb01eld. The SLM 72 \f1.4. Experimental Setup and Pulse shaper Figure 1.27: Liquid crystal molecules are represented as elliptical rods. (A) shows the anisotropic optical property of nematic liquid crystals. It has two refractive indices along and perpendicular to the averaged molecular orientation. (B) shows the equilibrium orientation of liquid crystal molecules. Figure C shows the liquid crystal orientations under external static electric \ufb01eld with voltages applied. a\ufb00ects the amplitude and spectral phase of the light in a discrete fashion. The amplitude and phase is independently adjustable for each SLM pixel. But within one pixel, the light experiences the same amplitude and phase. Mathematically, the amplitude mask A(\u03c9) and \u03c6(\u03c9) functions are stepwise. The CRI SLM-128 and CRI SLM-640 are used. In our experiments, they both have a pixel width of 100\u03bcm. Properties of Liquid Crystal The core elemental of the SLM is a voltage-controlled nematic liquid crystal (NLC) array. Nematic is a phase of the liquid crystal (LC), where LC molecules have directional order but do not have long range periodicity. The NLC molecule has a rod-like shape and is macroscopically anisotropic. For an optical wave, NLC media exhibit two refractive indices no and ne . This property allows the polarization rotation of light when it passing through NLC media. In the equilibrium state, the orientation of NLC shows a statistically directional order. A better orientation alignment can be achieved 73 \f1.4. Experimental Setup and Pulse shaper Figure 1.28: When the light passes through liquid crystal molecules, it sees the e\ufb00ective refractive index as a linear combination of no and ne . It is dependent on the molecular orientation. \u03b1 is the angle between the light propagation direction and molecular alignment direction. (A) shows the light propagation direction and liquid crystal molecular alignment. (B) shows the e\ufb00ective refractive index that the light sees on the refractive index sphere. 74 \f1.4. Experimental Setup and Pulse shaper when molecules are under an external electric \ufb01eld. Figure 1.27 shows this property of NLC. The phase change introduced by the SLM is connected with the optical path and refractive index. It is given by \u03b4\u03c6 = 2\u03c0 \u03b4n\u00b7l \u03bb where l being the length of the NLC media, \u03bb being the wavelength of light and \u03b4n being the change of refractive index, which is a function of the average orientation of liquid crystal molecules (\ufb01gure 1.28). Since the orientation of NLC molecules can be a\ufb00ected by external static electric \ufb01elds and the refractive index is dependent on the orientation of NLC molecule, the phase is therefore controlled by the external voltage applied on the liquid crystal array. Since the NLC is also bifringent, when it changes the spectral phase of the light, it also rotates the polarization. This polarization rotation can be used for amplitude shaping with polarizers. However, the spectral phase change and the polarization change are coupled for a single SLM mask. The spectral phase and polarization cannot be shaped separately with only one SLM mask. This disadvantage can be compensated by using a second liquid crystal mask. Two masks introduce the same amount of phase shift but rotate the polarization in the opposite direction. The net e\ufb00ect is then a shift in spectral phase without polarization rotation. Calculation on Speci\ufb01cations of Optics Before building a pulse shaper, the parameters of the optical elements must be considered. Since the spatial light modulator is the central part of a pulse shaper, the choice of gratings and focusing lens\/mirrors should \ufb01t the speci\ufb01cation of the SLM and the input beam size. For example, the CRI SLM-640 (SLM) has a pixel size of 100\u03bcm, and the input beam has a diameter of 5mm (an iris is set in front of the pulse shaper entrance to down size the beam). The focus spot can be estimated by equation: d = 1.22f\u03bb\/D (1.53) with D being the input beam diameter, \u03bb being the wavelength of light and f being the focal length. If the central wavelength is 800nm and we assume 75 \f1.4. Experimental Setup and Pulse shaper the focus spot is equal to the pixel width of the SLM, the calculated focus length f is 50cm. This means 50cm focus length mirrors or lenses should be used as the collimating element. The next step is the selection of gratings. The main consideration is that the width of the dispersed broad band pulse should \ufb01t the width of SLM. Therefore, the ideal dispersing ability of the grating depends on the SLM window width and the laser bandwidth. The width of the CRI SLM-640 SLM window is 5 cm. The maximal allowed angular dispersion width can be calculated as : \u03b8 = w\/f (1.54) with w being the width of SLM. The calculated maximal allowed angular dispersion is 0.1 radians. The laser bandwidth out of the Spit\ufb01re Pro is 40nm (FWHM) with central wavelength of 800nm, the grating should disperse the spectrum such that the angular spread equals the maximal allowed angular dispersion of 0.1 radians. The solution can be found using the grating equation: sin \u03b8d = n\u03bb\/d\u0004 \u2212 sin \u03b8i (1.55) with \u03b8i ,\u03b8d being the incident and di\ufb00racted angle respectively, n being the order of grating and d\u0004 being the grating constant. The calculable form is: \u03b8 = arcsin( n(\u03bb \u2212 B\/2) n(\u03bb + B\/2) \u2212 sin \u03b8i ) \u2212 arcsin( \u2212 sin \u03b8i ) \u0004 d d\u0004 (1.56) with B being the total wavelength bandwidth of the pulse shaper. It should be bigger than the bandwidth of the laser pulses so as to let the wings of spectrum go through the SLM window. A factor of three is good: with 40nm FWHM laser bandwidth, B will have the value of 120nm. If one assumes that the incident angle of light on the grating is \u03c0\/6 radian and the grating is working in \ufb01rst order (n=1), equation (1.56) leads to the selection of 800 grooves per mm grating. Because 800 grooves per mm grating blazed for 800nm was not available at the time when the pulse shaper was built, gratings of either 600 grooves per mm or 1200 grooves per mm were used in our experiments. 76 \f1.4. Experimental Setup and Pulse shaper Figure 1.29: (A) shows the top view of folded pulse shaper design. (B) shows the side view of folded pulse shaper design. This design requires only one grating and one lens compared to original design shown in \ufb01gure 1.26. It reduces the alignment e\ufb00ort on angle and pitch adjustment. 1 is the input\/output mirror, 2 is the grating, 3 is the collimating mirror, 4 is the SLM and 5 is the adjustable mirror that mounted behind the SLM. Assembly of The Pulse Shaper The assembly and adjustment of optical elements of the pulse shaper should ful\ufb01ll the corresponding mathematical functions as expression (1.52) shows. This provides guidelines for pulse shaper adjustment. The grating pairs and collimating lenses should perform the forward and inverse Fourier transform by placing the gratings at the focal distance of the lenses. The SLM should also be capable of changing both amplitude and phase for each frequency component. First of all, the SLM has to be put in the Fourier plane. The forward Fourier transform introduced by the left side grating and collimating lens (\ufb01gure 1.26(A)) should be canceled by the inverse Fourier transform introduced by the right side (\ufb01gure 1.26(C)) optical elements. The distance between lens and gratings should be equal to the focal distance of lens, and the gratings of both sides should be at the same angle. To achieve this, careful alignment of gratings and lenses is required. With the setup shown in \ufb01gure 1.26, there are two gratings and two lenses in the setup. The po- 77 \f1.4. Experimental Setup and Pulse shaper sition and pitch of these four optical elements have to be adjusted and pair compensated, which is not easy. As a result, an alternative design was created to simplify the pulse shaper setup by using a re\ufb02ective geometry. If a mirror is used after the SLM, light can be re\ufb02ected back to the same collimating lens and grating. The back re\ufb02ection guarantees the light goes through the same grating at the same angle, the same lens and the same distance. In this geometry, the only adjustable parameter is on the distance between lens and grating and the angle of the grating. This reduces the alignment of previous four optical elements down to alignment of two. The new design is shown in \ufb01gure 1.29. A pulse shaper of 128 pixels SLM (CRI SLM-128) was built according to this design. The folded design occupies a smaller space on optical table than the original design (\ufb01gure 1.26), because it is only 2f in length (twice the focus length). The length of the pulse shaper can be further reduced to 1f if a focusing mirror is used instead of a lens. Figure 1.30 shows the setup of a folded pulse shaper based on mirror. A pulse shaper with a 640 pixel SLM and 50cm focus distance was built according to this folded design, and it occupied 60cm by 50cm space of optical table (for photograph of this shaper, see \ufb01gure 1.3A). The folded pulse shaper design (\ufb01gure 1.30) is equivalent to the original 4f design(\ufb01gure 1.26). The advantages of this design are the compactness and elimination of transmissive lenses. As \ufb01gure 1.30 shows, it occupies only one focal length in terms of the total length of setup. Since a big SLM window width requires long focal length mirror given the same grating dispersion, the compact design avoids occupying excessive optical table space. For example, the CRI SLM-640 has a window size of 5 cm, and the calculated f is equal to 50cm. If the typical 4f geometry is used, it will occupy a space of 2 meters length, which means nearly one third to one half of the optical table. Moreover, transmissive lenses introduce dispersion into broad band pulses that has to be corrected afterward, whereas the design with re\ufb02ective mirror avoids dispersion. The optical alignment procedure of the pulse shaper can be found in appendix B.1. 78 \f1.4. Experimental Setup and Pulse shaper Back mirror A SLM Grating M Output Input Grating CM B SLM CM Input 1 1 M 2 2 Output E C 1 2 3 4 D Figure 1.30: The above \ufb01gures show the setup of a folded pulse shaper with a focusing mirror. The grating in this setup is either 600 or 1200groves\/mm, and the cylindrical mirror f = 50cm, and CRI SLM-640 has window size about 5cm. (A) shows the top view of the pulse shaper. (B) shows the side view of this pulse shaper. Insets (C) to (E) shows the light pro\ufb01le on corresponding optical elements. The alignment of the pulse shaper can be found in appendix B. A photograph of the pulse shaper of this schematic is shown in \ufb01gure 1.3A. 79 \f1.4. Experimental Setup and Pulse shaper Spatial Light Modulator Calibrations The ideal input parameters of a pulse shaper are the amplitude and phase. However, the SLM works on voltage. To make the pulse shaper functional, the calibration of voltage vs. phase is necessary. This is done by measuring the transmittance of polarized broadband light. The detailed procedure is included in appendix B.2 After measurement on the transmittance vs. voltage, the phase can be calculated from transmission through equation (1.57) T = cos2 (\u03c6\/2) (1.57) with T being the transmission and \u03c6 being the phase. This equation can be recast into: \u221a \u03c6 = 2 arccos T + k \u00b7 2\u03c0 (1.58) with k being an integer number to re\ufb02ect the multi value property of phase. The transmission vs. voltage curve then can be converted into a continuous phase vs. voltage curve. A polynomial \ufb01tting is used to obtain an analytical form of such a relation, represented as \u03c6(V ), and an inverse function for the voltage vs. phase V (\u03c6) can be found as well. For a dual-mask SLM, such as CRI SLM-640, calibrations have to be done for both masks. When the voltage vs. phase calibrations V (\u03c6) for both masks of the CRI SLM-640 are ready, the next step is to convert the amplitude and phase values into voltage value. For a given pair of amplitude A (A is the square root of the intensity I) and phase shaping \u03c6, the voltage on two masks V1 and V2 can be calculated using the following expressions: V1 = V (arccos(A) \u2212 \u03c6) (1.59) V2 = V (arccos(A) + \u03c6) (1.60) Expression (1.59) and (1.60) can be used to construct the voltage array mask for the masks of the SLM. As the experimental implementation, a Labview script was programmed to automatically convert the amplitude and phase into voltages for both masks. 80 \f1.4. Experimental Setup and Pulse shaper 1.4.4 Pulse Characterization Pulse characterization constituted an important part of the experiments in this thesis. Since the result of the broad band CARS experiment depends on the phase as well as the amplitude pro\ufb01le of the broad band pulse, a careful characterization of pulse pro\ufb01les is needed for the success of the experiment. There were two pulse characterization methods used in this thesis work: Frequency Resolved Optical Gating[78] (FROG) and Multi-photon intrapulse interference phase scan (MIIPS) [79]. The FROG technique was initially invented by Trebino and coworkers[78, 80] to recover the phase information of an ultrafast pulse. The idea of FROG is to use an iterative phase-intensity retrieving algorithm on a two-dimensional time-frequency second harmonic spectrogram to recover the phase and intensity information of the unknown pulse. Figure 1.31 shows a typical FROG device setup. The detailed discussion of the FROG technique can be found on literature [78, 80]. For the experiments of this thesis, the phase information of an unknown pulse was obtained through the FROG technique. The MIIPS technique achieves the pulse characterization through phase compensation. It was invented by Dantus and coworkers [79]. The unknown pulse is coupled into a pulse shaper and then frequency doubled in a nonlinear crystal. The second harmonic signal is measured by a spectrometer. A sinusoidal phase mask is applied to the unknown pulse through the pulse shaper and scanned across the spectrum of the pulse. The pro\ufb01le of the corresponding SHG spectrum is used to deduce the second derivative of the spectral phase of the unknown pulse and create the compensation phase mask. MIIPS characterization works iteratively to obtain a transform-limited pulse. The detailed implementation can be found in the literature[79]. In this thesis work, a Labview program was created to implement the scanning of the sinusoidal phase mask and recovery of the phase pro\ufb01le. The FROG technique was proposed earlier and it can work without a pulse shaper. The MIIPS technique can achieve a more precise phase characterization than FROG (FROG gives a precision of about 0.05 radian, 81 \f1.4. Experimental Setup and Pulse shaper FROG software Pulse to be measured Camera Spectrometer Beam splitter E(t\u2013W) BBO crystal D E(t) Figure 1.31: This \ufb01gure shows a FROG setup. The unknown ultrafast laser pulse is beam split into two pulses. One pulse is delayed by \u03c4 using a retrore\ufb02ector on translation stage. Then two pulses are combined at a nonlinear crystal for the second harmonic generation (thin type-I BBO cut at 29.2\u25e6 for 800nm). Scanning \u03c4 and recording spectra of the second harmonic signal to obtain the two-dimensional spectrogram (also known as the FROG trace). Then the trace is analyzed by FROG3 software (Femtosoft technology) to give amplitude and phase information of unknown pulse. 82 \f1.4. Experimental Setup and Pulse shaper whereas MIIPS can reach precisions better than 0.01 radian). Since the pulse shaper has become a common instrument in modern ultrafast laser labs, MIIPS requires only an additional second harmonics generation setup, therefore it is simpler to implement for a lab with a functional pulse shaper. A combination of these two methods was used in the thesis work. A FROG and a MIIPS setup were built near the output location of the pulse shaper. 1.4.5 Generation and Detection of CARS Signal For single pulse CARS experiments, the generation of signal can be simply achieved by focusing on the sample, if the focusing condition satis\ufb01es the phase matching requirement (see section 3.5). A tight focus lens or microscope objective is normally used for single pulse CARS. For the BOXCARS geometry CARS experiment, there are two strict requirements for generating detectable signals: \ufb01rst, all beams should spatially overlap on the sample, and second, excitation pulses should overlap in time. This temporal overlap requirement is di\ufb00erent in the femtosecond laser CARS experiment than in CARS with narrow band lasers. For narrow band excitations, the temporal overlap requirement is relaxed, if not automatically satis\ufb01ed. The following subsections shows some useful simple techniques in femtosecond CARS signal generation. Spatial and Temporal Overlap Adjustment After placing optical elements on the optical table according to an experimental scheme, a photo diode (DET 210 Thorlabs) is placed in the location of samples and used to detect excitation pulses after attenuation. The signal from the photo diode is displayed on an oscilloscope (TDS 3034B Tektronix). The time of attenuated pulses can be measured with the precision of 0.5ns (about 15cm in distance). The length of optical path of beams can be adjusted by either retro re\ufb02ectors in the setup or the position of mirrors. After pre-synchronization, the next step is to achieve spatial overlap. A business card with a small hole (about 50-100\u03bcm) can help alignment. It is mounted on a rigid frame near the sample of CARS experiment. A mirror on 83 \f1.4. Experimental Setup and Pulse shaper a \ufb02ipper is used to divert the focusing beams towards the mounted business card. The card is placed at the focal plane of the focusing element. Optical paths of all three beams are adjusted to let the attenuated beams passing through the small hole. An infrared detection card or an infrared viewer is used to view the beams after the hole. This procedure can guarantee good spatial overlap. The temporal overlap can be obtained by using a nonlinear crystal to generate a \u201csimulated signal\u201d at the CARS frequency. After the presynchronization step, the pulse delay di\ufb00erence is within 0.5ns. The femtosecond time scale synchronization is done by adjusting the motorized translation stages. A point worth noting is that the axis of the translation stage should be parallel to the incident beam in order to avoid spatial walk-o\ufb00 during the time delay scanning. Such walk-o\ufb00 can harm the spatial overlap at the focus spot which considerably reduces the signal. In the experiments of this thesis, a 100\u03bcm second harmonic BBO crystal cut at angle of 29.2\u25e6 (for 800nm second harmonic generation) was used for pulse synchronization. By placing the BBO crystal at the sample position, the time delay between two beams is scanned to \ufb01nd the sum-frequency or nonresonant four-wave-mixing signal from incident laser pulses. The time delay of two CARS excitation pulses are adjusted to ensure all three pulses arrive at sample at the same time. Signal Filtering and Detection The nonlinear crystal that is used for synchronizing the pulses can also be used to generate the four-wave-mixing (FWM) signal at anti-Stokes frequency. The FWM signal at CARS frequency can be used for detector alignment. In non-collinear geometry such as BOXCARS, the FWM signal should have the same spatial propagation direction as CARS signal generated by samples (see section 1.3, phase matching section). Therefore aligning the strong, sometimes even visible FMW signal to the spectrometer can give a good pre-alignment for the actual signal. In the experiments a CCD detector (Andor DV400) on a spectrometer (McPherson 2035) was used to detect 84 \f1.5. Structure of Ph.D. Thesis the signal. The scattering of intense excitation beams from samples increase the background in the CARS spectrum. Spatial \ufb01ltering of the signal is then needed. In experiments, an iris was used to block o\ufb00 the residual excitation beams after the sample. It was placed in such way that the the background was minimized and CARS signal was maximized. After the spatial \ufb01ltering iris, a dielectric short-wave-pass \ufb01lter (Semrock) was used to further improve the signal to noise ratio by \ufb01ltering out the residual scattered excitation beam. In the situation of collinear geometry, since spatial \ufb01ltering is not possible, multiple short-wave-pass \ufb01lters are often used to e\ufb00ective block the excitation beams. Polarization techniques that reduce the non-resonant background can be used to improve signal quality as well. In CARS experiments with BOXCARS geometry, the polarization of probe pulse can be rotated to 90\u25e6 related to the polarization of pump and Stokes pulses, which leads to three times reduction on the strength of non-resonant background compared to that of three pulses of the same polarization. This is because \u03c7(3) for isotropic samples has \u03c7xxxx = 3\u03c7xxyy relation[71], with \u03c7xxxx referring to the component of \u03c7(3) tensor when all pulses have the same polarization and \u03c7xxyy referring to the component of \u03c7(3) tensor when the pump and the Stokes pulses have the same polarization, and the probe pulse and anti-Stokes \ufb01eld are 90\u25e6 to it. 1.5 Structure of Ph.D. Thesis As a truth in science, every method has its own limitations. The technique of CARS is not an exception. For example, CARS with broad band pulses lacks spectral resolution, which is seen as a serious drawback to its spectroscopic application. The non-resonant background a\ufb00ects the CARS spectrum adversely, which also limits its application. The emphasis of this PhD thesis is on developing new methods to improve the performance of CARS with broad band pulses. The investigations have been done with the combination of broad band laser pulses and the pulse shaping technique. 85 \f1.5. Structure of Ph.D. Thesis The PhD thesis is presented in the following structure. The results of the experiments during my PhD study are presented in chapters 2 to 5. In chapter 2, the technique of Noise Auto-correlation Spectroscopy with Coherent Raman Scattering is presented. This is a single pulse CARS approach with the utilization of spectral noise across full pulse bandwidth. In chapter 3, an optical processing experiment of optical correlation on CARS is presented. It can obtain a high spectral resolution CARS spectrum from optical interference of broad band pulses and CARS signal. The method of complete characterization of molecular vibrations is presented in Chapter 4. This method can recover both amplitude and phase of laser-induced coherent vibrations. 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White, Journal of the Optical Society of America B-Optical Physics 11, 2206 (1994). 91 \fChapter 2 Noise Auto-correlation Spectroscopy with Coherent anti-Stokes Raman Scattering 2.1 Motivation Noise Auto-correlation Spectroscopy with Coherent anti-Stokes Raman Scattering (NASCARS) is the method that will be introduced in this chapter. In section 1.3, expression (1.2) shows that the CARS signal generation in the frequency domain is a convolution between the probe \ufb01eld E(\u03c9) and the vibrational coherence R(\u03a9). The vibrational coherence R(\u03a9) contains the pro\ufb01le of vibrational resonances according to the Lorentzian model equation (1.31). The purpose of CARS spectroscopy is to recover R(\u03a9) from the detectable CARS signal. In narrow band CARS or the multiplex CARS method, a narrow band probe pulse is used. With a narrow bandwidth probe pulse, the CARS spectrum has the same pro\ufb01le as the spectrum of the vibrational coherence (including non-resonant background). However, when a broad band coherent probe pulse is used, the CARS signal not only re\ufb02ects the vibrational coherence, but also re\ufb02ects the pro\ufb01le of the probe pulse. Therefore, the CARS spectrum cannot be taken as a direct indication of resonant level positions without further interpretation. Figure 1.20 0 A version of this chapter has been published as Xiaoji G. Xu, Stanislav O. Konorov, John. W. Hepburn and Valery Milner \u201cNoise Auto-correlation Spectroscopy with Coherent anti-Stokes Raman Scattering\u201dNature Physics Vol.4 No.2 page 125-129, 2008 92 \f2.1. Motivation C shows considerable di\ufb00erence in CARS spectra between sinusoidal phase shaping and \u03c0 phase step shaping. The CARS spectra dependence on the probe pulse raises a question: under broad band probe pulse condition, how can the vibrational coherence information be recovered from the broad band CARS signal? This chapter will give one answer to this question. As discussed in section 1.3, the vibrational coherence R(\u03a9) is not directly measurable by the spectrometer. But the CARS signal as well as the optical \ufb01eld of probe pulse is a directly measurable quantity. From the information \ufb02ow point of view, the information about the vibrational coherence is transferred to the measurable CARS signal through the anti-Stokes scattering of the probe pulse. The CARS spectrum with a narrow band probe pulse (\ufb01gure 2.1B) re\ufb02ects the position and linewidth of the vibrational resonances. The CARS spectrum with a broad band probe pulse (\ufb01gure 2.1A) is broad and structureless. Useful information about the resonant levels is not e\ufb00ectively transferred by the broad band pulse through measurable CARS signals. This is a natural result of the fact that CARS signal is a convolution between the probe \ufb01eld and the vibrational coherence in the frequency domain. A closer look at the time domain gives an alternate but equivalent explanation. The vibrational coherence R(t) interacts with the probe pulse according to equation (1.37). While R(t) has a long lasting time behavior, the transform-limit probe pulse only overlaps with a small part of R(t) (\ufb01gure 2.1C), whereas the narrow band probe pulse can overlap with the vibrational coherence at all time (\ufb01gure 2.1D). As a result, only a small part of the time domain response of the vibrational coherence is transferred to the CARS \ufb01eld when the probe pulse has short duration, leading to the loss of structural information of molecules in the CARS spectrum. The time domain analysis indicates a way to solve the problem. In order to obtain good information transfer from the vibrational coherence to the CARS spectrum, the probe pulse should have a long duration that can cover the whole time domain behavior of the vibrational coherence. However, the probe pulse having a long time duration is only a necessary requirement to the solution but not a su\ufb03cient one. Chirping or introducing phase functions to the probe pulse can extend the pulse duration and create sharp features 93 \f2.1. Motivation 6 Intensity (AU) A B 4 2 0 700 720 740 760 780 Wavelength (nm) 800 700 720 740 760 Wavelength (nm) 780 800 Intensity (AU) 1 C 0.8 D 0.6 0.4 0.2 0 0 1 Time (ps) 2 3 0 1 2 3 Time (ps) Figure 2.1: These \ufb01gures show a comparison between a CARS spectrum using a transform-limited broad band probe pulse (300cm\u22121 bandwidth) (A), and a narrow band probe pulse (3cm\u22121 bandwidth) (B). (C) and (D) show the comparison in the time domain of CARS generation by a transformlimited probe pulse (thick red curve in (C))and a narrow band probe pulse (thick red curve in (D)) overlapping with the vibrational coherence (thin blue curve in both (C) and (D) ). 94 \f2.1. Motivation A Intensity (AU) B 700 740 780 820 700 740 780 820 Wavelength (nm) Wavelength (nm) D Intensity (AU) C 680 720 760 Wavelength (nm) 800 0 0.5 1 1.5 2 Time (fs) Figure 2.2: (A) shows the CARS spectrum using a positively chirped probe pulse. (B) shows the CARS spectrum using a negative chirped probe pulse. (C) shows the CARS spectrum from a noisy probe pulse. (D) in the time domain shows the vibrational coherence (blue thick line) and the noisy modulated probe pulse (red,thin line). The vibrational coherence in these \ufb01gures is the same as that of \ufb01gure 2.1 and the following \ufb01gure 2.3 . 95 \f2.1. Motivation in the CARS spectrum, but they require additional interpretation as well as the exact knowledge of the probe pulses. As an example, \ufb01gure 2.2 A and B show spectra of CARS signal generated by a positive chirped and a negative chirped probe pulse. Firstly, the spectra have di\ufb00erent shapes from the vibrational coherence (\ufb01gure 2.1B). Secondly, the CARS spectrum created from a chirped probe pulse is clearly dependent on the sign of the chirp. There have been some studies [1, 2] done on \ufb01nding a speci\ufb01c phase shape for broad band probe pulses such that the corresponding CARS spectrum can re\ufb02ect the resonance structure. In Oron et. al.[1] a \u03c0 phase step and a 0.5\u03c0 phase step pulse shaping pattern were used to resolve the resonances in a broad band CARS spectrum. However, such an approach requires exact and accurate pulse shaping of the probe pulse. In this chapter, an alternative approach which does not resort to speci\ufb01c pulse shapes of the probe pulse is presented. This approach is to introduce uncorrelated spectral noise into the broad band pulse and measure the correlation between spectral peaks in the CARS spectrum. The \ufb01gure 2.2C shows the CARS spectrum from a noisy probe pulse. The sharp features in the spectrum result from the presence of vibrational resonances and the long time duration component of the probe pulse. Figure 2.2D shows the shape of the vibrational coherence and a noise modulated probe pulse in the time domain. The noise modulated probe pulse has a long time duration that can e\ufb00ectively overlap with the vibrational coherence R(t). Therefore, it satis\ufb01es the above mentioned probe pulse requirement. However, the generated noise CARS spectrum contains both the pro\ufb01le of vibrational coherence and the noisy pattern of the probe pulse. It cannot be used directly. However, as will be shown in the following paragraphs, the autocorrelation of the noisy CARS spectrum can re\ufb02ect the pattern of the vibrational coherence, if the patterns are uncorrelated. Consider the intensity of the time domain anti-Stokes \ufb01eld: \u2217 (t) Ias (t) = Eas (t)Eas (2.1) 96 \f2.1. Motivation From equation (1.37) of section 1.3, the expression of the time domain \ufb01eld Eas (t) can be treated as C \u00b7Epr (t)R(t). The product of vibrational coherence R(t) and the probe \ufb01eld Epr (t) times a constant C, which can be assumed as 1, since it is the pro\ufb01le of the signal \ufb01eld, not the total amount of CARS signal that is interesting. Then the time domain intensity of the anti-Stokes becomes: \u2217 (t) Ias (t) = R(t)R\u2217 (t)Epr (t)Epr (2.2) The right hand side of equation(2.2) can be separated into two parts: the intensity of the time domain vibrational coherence, R(t)R\u2217 (t), and the inten\u2217 (t). If the probe pulse is noise modulated, sity of the probe \ufb01eld Epr (t)Epr \u2217 (t) term then contains a narrow band the Fourier transform of Epr (t)Epr central frequency component. The Fourier transform of the left hand side of the equation (2.2) gives the autocorrelation of the frequency domain spectrum of the amplitude and the spectral phase . f f t{Ias (t)}(\u03a9) = \u0003 \u221e \u2212\u221e E \u2217 (\u03c9)E(\u03c9 + \u03a9)d\u03c9 (2.3) The Fourier transform of the right hand side of equation(2.2) represents the convolution of the Fourier transform of the time domain intensity of the vibrational coherence R(t)R\u2217 (t) and the time domain intensity of the probe \u2217 (t) according to equation (2.4). pulse Epr (t)Epr f f t{Ias (t)}[\u03a9] = f f t{R(t)R\u2217 (t)}[\u03a9] \u000f \u2217 f f t{Epr (t)Epr (t)}[\u03a9] (2.4) In a similar fashion to equation (2.3) for the CARS intensity, the f f t{R(t)R\u2217 (t)} corresponds to the autocorrelation of the vibrational coherence spectrum of amplitude and phase (\u201cof amplitude and phase\u201d means it is a complex quantity rather than a real quantity) by f f t{R(t)R\u2217 (t)}[\u03a9] = \u000e\u221e \u2212\u221e R \u2217 (\u03c9)R(\u03c9 + \u2217 (t)} corresponds to the autocor\u03a9)d\u03c9 . The probe pulse part f f t{Epr (t)Epr \u2217 (t)}[\u03a9] = relation of the probe pulse spectrum of amplitude and phase f f t{Epr (t)Epr \u000e\u221e \u2217 \u2212\u221e Epr (\u03c9)Epr (\u03c9 + \u03a9)d\u03c9. Numerical simulations can better illustrate the relation between the 97 \f2.1. Motivation Intensity (AU) 2 2 A B 1.5 1.5 1 1 0.5 0.5 0 0 -800 -400 0 400 800 -800 Frequency (cm-1) -400 0 400 800 Frequency (cm-1) 3 4 Intensity (AU) 2.5 D C 3 2 1.5 2 1 1 0.5 0 -800 -400 0 400 Frequency (cm-1) 800 0 -800 -400 0 400 Frequency (cm-1) Figure 2.3: (A) shows the plot of the Fourier transform of the probe pulse intensity in time of two low amplitude phase noise patterns (red and blue). (B) shows similar plots but with two high amplitude spectral phase noise patterns (6 times higher than that of (A)). (C) shows the frequency domain Fourier transform of the vibrational coherence intensity R(t)R\u2217 (t), the vibration level spacing is indicated by the vertical dashed lines. (D) shows the Fourier transform of the CARS intensity. Blue dashed curve is from one low amplitude noise pattern of (A). Red continuous line is from one high amplitude noise pattern of (B)). 98 800 \f2.1. Motivation noisy probe pulse and the vibrational coherence than equations. \ufb01gure 2.3 shows the autocorrelation of the probe pulse spectrum of amplitude and phase and the autocorrelation of the vibrational coherence spectrum of amplitude and phase. From \ufb01gure 2.3A and 2.3B, one can \ufb01nd that the phase noise in the probe pulse gives a narrow band central peak in the frequency domain autocorrelation. The high noise level in the probe pulse gives a pedestal in the autocorrelation spectrum. The total autocorrelation of CARS spectrum (expression (2.3)) is shown in \ufb01gure 2.3D. It is a convolution between the autocorrelation of the vibrational coherence spectrum (\ufb01gure 2.3C) and the autocorrelation of the probe pulse spectrum (\ufb01gure 2.3B). Because of the convolution, the narrowness of the central peak of \ufb01gure 2.3B determines the resolution of total autocorrelation spectrum of \ufb01gure 2.3D. However, as \ufb01gure 2.3D shows, in addition to the peaks that correspond to the autocorrelation of complex vibrational coherence spectrum (vertical lines in \ufb01gure 2.3D), there are also additional side peaks that come from the residual correlation of spectral noise of the probe pulse. This is due to the fact that no matter how random the probe pulse noise is, the \ufb01nite bandwidth or duration of the probe pulse always contains residual correlations. To solve this problem, averaging over multiple noise patterns is introduced. There is also a pedestal in the autocorrelation spectrum of the probe pulse when the amplitude of noise is low (\ufb01gure 2.3A). Because of the convolution, the pedestal in the autocorrelation of the probe pulse also creates a problem for the \ufb01nal autocorrelation of the spectrum (see \ufb01gure 2.3D). The autocorrelation pedestal originates from the central short duration part of the probe pulse in the time domain (the pro\ufb01le of pulse is similar to \ufb01gure 2.4). When the spectral phase noise is high, the time domain pulse is dispersed into irregular pulse trains and the central short duration part is eliminated, leading to a low pedestal in the Fourier transform (\ufb01gure 2.3B). For proof of principle NASCARS experiment with BOXCARS geometry, a separate probe pulse is used. It is possible to use the pulse shaper to introduce high amplitude noise into the probe pulse to remove the pedestal. However, for the proposed single pulse NASCARS experiment (see below), 99 \f2.1. Motivation since the pump\/Stokes and probe pulses are uni\ufb01ed into one single excitation pulse to maintain the short duration central part for the impulsive vibrational coherence preparation (\ufb01gure 2.4). The high noise amplitude approach is not applicable to the single pulse NASCARS. To solve this problem, subtraction between consecutive noise CARS spectra is used before numerical autocorrelation. Such subtraction is e\ufb00ective for both BOXCARS geometry NASCARS and single pulse NASCARS. The single pulse NASCARS experiment utilized a broad band excitation pulse of spectral noise of low amplitude to coherently excite the vibrational coherence and probe it. When a broad band pulse contains spectral noises of low amplitude, its time domain representation shows a short duration central peak and a long duration tail of irregular pulse trains (\ufb01gure 2.4). The long duration tail of the uni\ufb01ed pulse can serve as the probe pulse of NASCARS, and the central short duration part serves as the impulsive excitation. The pulse shape of single pulse NASCARS is similar yet di\ufb00erent to that of the single pulse CARS method mentioned in section 1.2 (see \ufb01gure 1.12). In both single pulse experiments, the short duration envelope in the time domain creates the vibrational coherence, and the \ufb01eld of the long tail probes the prepared vibrational coherence. The di\ufb00erence between these two single pulse method is primarily in the probing function. In NASCARS, the probing \ufb01eld is created by the spectral noise of low amplitude, and the spectral noise modulation exists across all parts of the spectrum. In single pulse CARS, the probe \ufb01eld is a narrow band frequency component and speci\ufb01cally allocated at the blue edge of the spectrum. In the frequency domain representation, the autocorrelation of the excitation pulse of single pulse NASCARS contains a pedestal and a central peak of narrow bandwidth. The autocorrelation pedestal covers the bandwidth that is accessible for NASCARS. The central peak of narrow bandwidth in the autocorrelation spectrum determines the spectral resolution (the autocorrelation of excitation pulse in single pulse NASCARS has the same pro\ufb01le shown in \ufb01gure 2.3A). In the above derivation, the autocorrelation of the CARS \ufb01eld is treated as \u000e\u221e \u2212\u221e E \u2217 (\u03c9)E(\u03c9 + \u03a9)d\u03c9 . In the actual experimental measurement, the 100 \f2.1. Motivation 8 Impulsive excitation part Intensity (AU) 7 6 5 Vibration coherence 4 3 2 Probe part 1 0 0 0.5 1 1.5 Time (ps) Figure 2.4: This \ufb01gure shows the time domain representation of a single pulse NASCARS excitation pulse. The low level noise broad band pulse in the time domain has two parts (the high-lighted boxes), the coherent central part and the noise tail part. The coherent central part is capable of generating vibrational coherence(dashed line). The central part is conserved from realization to realization. The continuous thick curves (red and blue) show two of such random low level noisy pulse. The dashed curve represents the vibrational coherence in time. 101 \f2.1. Motivation autocorrelation is done based on the CARS spectrum as \u000e\u221e \u2212\u221e I(\u03c9)I(\u03c9+\u03a9)d\u03c9. The autocorrelation of the CARS spectrum and the autocorrelation of the CARS \ufb01eld of amplitude and phase both can yield the vibrational level spacing of the sample. The \ufb01rst experiment was done in a BOXCARS geometry using a pulse shaper to introduce high spectral noise to a probe pulse, and then the difference between CARS spectra of two consecutive CARS spectra was measured. An autocorrelation of the di\ufb00erence of CARS spectra was taken and averaged. The averaged autocorrelation spectrum of many di\ufb00erent random noise probe pulse patterns shows the vibrational level spacings. After the proof of principle experiment of BOXCARS geometry, a single pulse CARS experiment was demonstrated. We found a convenient way of creating low level noise modulated pulse from a regenerative ampli\ufb01er by modifying the compressor grating system. With collinear focusing and proper signal \ufb01ltering, CARS spectra were obtained and consecutively subtracted. The di\ufb00erence of spectra follows the same treatment of autocorrelation and averaging. The experimental detail is shown in the article and method section. The single pulse NASCARS can reveal the vibrational level spacing of low wave numbers resonances. (< 400cm\u22121 ), limited by the bandwidth of the excitation broad band pulse. The single pulse NASCARS can give the spacing of the vibrational levels in a single pulse experiment. It inherits the compactness of the single pulse CARS technique and requires only a regenerative ampli\ufb01er laser system. Since the exact phase shape of noise is not required, single pulse NASCARS method can work without a pulse shaper. However, NASCARS recovers only the autocorrelation of the vibrational spectrum (2.3C) but not the spectrum itself (\ufb01gure 2.1B). The autocorrelation spectrum contains less structural information than the actual spectrum, e.g. the line width of resonances is hard to obtain through autocorrelation. Chapter 3 is going to address this autocorrelation problem and give a solution for obtaining the full spectrum using broad band noise pulse. 102 \f2.2. Method Content 2.2 2.2.1 Method Content Content Coherent anti-Stokes Raman scattering (CARS) with femtosecond laser pulses has become the method of choice in nonlinear optical spectroscopy and microscopy[3, 4]. As a third-order nonlinear process, femtosecond CARS exhibits high e\ufb03ciency at low average laser power. High sensitivity to molecular structure enables detection of small quantities of complex molecules[5, 6] and non-invasive biological imaging[7]. Temporal and spectral resolution of CARS is typically limited by the duration of the excitation pulses and their frequency bandwidth, respectively. Broadband femtosecond pulses, though advantageous for time-resolved CARS spectroscopy[8, 9], o\ufb00er poor spectral resolution. The latter can be improved by invoking optical[10, 11] or quantum[2, 12] interferences at the expense of increasing complexity of instrumentation and susceptibility to noise. Here we present a new approach to coherent Raman spectroscopy in which high resolution is achieved by means of deliberately introduced noise. The proposed method combines the e\ufb03ciency of a coherent process with the robustness of incoherent light, and does not require any temporal scanning or spectral pulse shaping commonly employed by the frequency-resolved spectroscopic methods with ultrashort pulses. In CARS, pump and Stokes photons of frequencies \u03c9p and \u03c9S , respectively, excite molecular vibrations at frequency \u03a9 = \u03c9p \u2212 \u03c9S (Figure a). A probe photon at \u03c90 is scattered o\ufb00 the coherent vibrations generating the anti-Stokes signal at frequency \u03c9 = (\u03c90 +\u03a9). Special care is usually taken to preserve the coherence of laser pulses as it determines the accuracy of a spectroscopic measurement. The latter can be improved by means of the pulse shaping technique[1, 13] which modi\ufb01es the amplitudes and phases of the spectral constituents of the pulse[14] (Figure 2.2.1b(i)). It enables selective excitation[2, 12] or selective probing[10, 11] of separate vibrational modes on the frequency scale narrower than the overall pulse bandwidth. Selective excitation is based on the coherent control[15] of nonlinear optical processes [16], whereas selective probing employs the idea of multiplex CARS[7] in 103 \f2.2. Method Content which a small part of the pulse spectrum is modi\ufb01ed (in amplitude, phase or polarization) and serves as a narrowband probe. Both approaches rely on the e\ufb00ects of quantum or optical interference, and are therefore sensitive to noise and de-coherence which often ruin the spectral and temporal integrity of the pulse. Using a narrow slice of the available pulse spectrum as a probe in multiplex CARS also means that higher resolution may only be obtained at the expense of the proportionally lower probe power and correspondingly lower signal. In this work we show that contrary to the common belief that spectral noise is detrimental to coherent spectroscopic measurements, it can be utilized for improving the resolution, e\ufb03ciency and robustness against unavoidable degradation of pulse coherence. In our new method of noise auto-correlation spectroscopy with coherent anti-Stokes Raman scattering (NASCARS) the laser-induced molecular vibrations are probed by a broadband pulse with intentionally randomized amplitude and phase. The vibrational resonances result in and are identi\ufb01ed through the appearance of intensity correlations in the noisy spectrum of coherently scattered photons. Due to the presence of Raman resonances, the spectral noise of the probe \ufb01eld is transferred to the spectrum of the scattered photons. While completely uncorrelated in the probe, the noise in the anti-Stokes \ufb01eld acquires strong correlations as a result of the molecular vibrational coherence. The latter assures that multiple Raman modes \u201cmap\u201d the same realization of the probe noise onto the di\ufb00erent spectral regions of the generated anti-Stokes spectrum, as shown schematically in Figure 2.2.1a. An auto-correlation of the noisy anti-Stokes spectrum corresponds directly to the auto-correlation of the Raman mode structure, thus revealing the vibrational beating frequencies of the medium. Even though the probe in NASCARS carries the full available spectral bandwidth of a femtosecond pulse, the resolution is determined by the much smaller frequency correlation length of the introduced noise, \u03b4\u03c9n . Utilization of the full bandwidth provides the ability to increase the resolution with no penalty in the available probe power and, therefore, with no direct reduction of the signal level. By its very nature, the method is not sensitive to the quality of the temporal and spectral pro\ufb01le 104 \f2.2. Method Content a \u012f\u0226n \u02260+\u020d2 CCD b Spectrometer \u02260+\u020d1 Sample SWP Sample LWP \u02260 (i) \u0226p (ii) (iii) Random diffuser \u0226S SLM \u020d2 Fibre \u020d1 OPA RGA C RGA cavity Figure 2.5: Interaction scheme for coherent anti-Stokes Raman scattering (CARS) and experimental arrangement for the detection of NASCARS signal. a, Pump and Stokes pulses (black) overlap in time and induce the coherent molecular vibrations. The broadband probe pulse (green) interacting with the vibrational energy levels \u03a91,2 generates the anti-Stokes light (red and blue). In NASCARS, the noise in the probe spectrum is imprinted onto the corresponding spectral regions of the anti-Stokes light. b, Diagrams of various experimental con\ufb01gurations. In (i), the random spectral noise is applied to the probe pulse by the spatial light modulator (SLM) in the pulse shaper con\ufb01guration. In (ii), the phase of the probe is randomized due to the inter-modal dispersion of a multi-mode optical \ufb01bre. In both cases, the pump and Stokes pulses are generated by the optical parametric ampli\ufb01er (OPA). In the single-pulse con\ufb01guration (iii), a di\ufb00user is introduced inside the compressor stage (C) of the regenerative ampli\ufb01er (RGA) system. Random scattering results in the partial de-coherence of the pulse required by NASCARS. The anti-Stokes spectrum is detected by the CCD-based spectrometer, and the auto-correlation is calculated by the computer. LWP, SWP - long- and short-wave pass \ufb01lters, respectively. 105 \f2.2. Method Content of the pulses, and can be implemented by simply destroying the coherence of a laser pulse, as demonstrated here. Noise and \ufb02uctuations in resonant \ufb02uorescence[17], scattered light[18] and number of trapped ultra-cold atoms[19] have been used to observe statistical properties of a medium but did not provide any spectroscopic information. NASCARS extends the idea of using noise correlations as a diagnostic tool to the domain of coherent nonlinear spectroscopy with ultrashort pulses. Noisy nanosecond lasers have been previously exploited in coherent Raman spectroscopy as a means of achieving time resolution shorter than the duration of the excitation pulses[20, 21]. The method of coherence observation by interference noise (COIN[22]) has been introduced for detecting the decay rates of electronic coherence, and applied to linear spectroscopy with narrow band picosecond pulses and to quantum state holography[23]. Unlike NASCARS, both approaches retrieve spectroscopic data from scanning the time delay between the noisy pulses. Here we show that the availability of a broad spectrum advances the method of noise-assisted spectroscopy towards e\ufb03cient scan-less single-beam frequency-resolved analysis of molecular vibrations. Consider the scheme depicted in Figure 2.2.1a with two Raman modes at frequencies \u03a91 and \u03a92 excited by the pump-Stokes pulse pair. The antiStokes \ufb01eld E(t), generated by the Raman scattering of the \u0010probe \ufb01eld E0 (t), \u0011 can be expressed as the real part of E(t) = E0 (t) \u00b7 e\u2212\u03b3t e\u2212i\u03a91 t + e\u2212i\u03a92 t , where for the sake of clarity we have neglected the non-resonant background, and assumed equal strength and decay rate \u03b3 for both vibrational modes. The experimentally observed anti-Stokes spectrum I(\u03c9) is the Fourier transform of the \ufb01eld correlation function GE (\u03c4 ), where \u0003 GE (\u03c4 ) = dtE(t)E \u2217 (t \u2212 \u03c4 ) = GE0 (\u03c4 )[ei\u03a91 \u03c4 + ei\u03a92 \u03c4 ]. (2.5) Here GE0 (\u03c4 ) is the correlation function of the modi\ufb01ed input probe \ufb01eld E0 \u2261 E0 \u00b7 e\u2212\u03b3t , i.e. the probe \ufb01eld multiplied by the exponential decay of 106 \f2.2. Method Content the vibrational coherence. Hence, \u0003 I(\u03c9) = d\u03c4 e\u2212i\u03c9\u03c4 GE0 (\u03c4 )[ei\u03a91 \u03c4 + ei\u03a92 \u03c4 ] = I0 (\u03c9 \u2212 \u03a91 ) + I0 (\u03c9 \u2212 \u03a92 ), (2.6) where I0 (\u03c9 \u2212 \u03a91,2 ) is the spectrum of E0 . Equation (2.6) shows that any amplitude noise in I0 is mapped onto the corresponding spectral region of the anti-Stokes spectrum I (that is, up-shifted by the corresponding Raman shift \u03a91,2 as schematically shown in Fig. a). Averaging over multiple noise realizations, we arrive at the expression for the noise auto-correlation for the measured anti-Stokes spectrum as a function of the frequency shift \u0394\u03c9: GI (\u0394\u03c9) = GI0 \u00b7 [2g(\u0394\u03c9) + g(\u0394\u03c9 + \u03b4\u03a9) + g(\u0394\u03c9 \u2212 \u03b4\u03a9)], (2.7) where \u03b4\u03a9 \u2261 \u03a92 \u2212 \u03a91 is the distance between the vibrational resonances, and we have assumed an uncorrelated probe noise with GI0 (\u0394\u03c9) \u2261 GI0 g(\u0394\u03c9) and g(\u0394\u03c9) being the line shape function peaked at \u0394\u03c9 = 0 and of width \u03b4\u03c9n . The two sidebands at \u00b1\u03b4\u03a9 in Eq. 2.7 illustrate the ability of NASCARS to retrieve the vibrational beating frequency from the frequency correlations in the noisy spectrum of the Raman-scattered light, with the resolution determined by the noise correlation length \u03b4\u03c9n . The required amplitude noise in the spectrum of E0 can be introduced by applying either amplitude or phase noise to the input probe \ufb01eld E0 . Numerical simulation of the NASCARS measurement with a phase-randomized probe \ufb01eld is shown in Fig. 2.6. In the time domain, the spectral noise breaks the initial short probe pulse into a long and random sequence of smaller pulses - an \u201cincoherent pulse train\u201d (Fig. 2.6b). In the presence of a long-lived vibrational coherence, this probe train generates a train of the corresponding anti-Stokes pulses. The anti-Stokes train is an exact replica of the original random sequence of the probe pulses with an additional periodic amplitude modulation superimposed on it by the vibrational \ufb01eld of the molecule. It is this amplitude modulation that introduces correlations in the otherwise uncorrelated noise in the observed anti-Stokes spectrum, shown in Fig. 2.6c. High spectral resolution is achieved when the probe train duration 107 \f2.2. Method Content Amplitude (a.u.) a b c 2\u028c 730 740 750 O\u0003\u0003(nm) 800 1000 1200 0 Frequency (cm-1) 1 2 3 4 Time (ps) 100 200 300 5 -100 0 Frequency (cm-1) Figure 2.6: Numerical simulations of the noise auto-correlation spectroscopy with CARS. a, the frequency bandwidth of the probe pulse, represented by the broad gaussian envelope, is much broader than the width of and the distance between the vibrational resonances of Toluene (black curve). White noise is applied to the spectral phase of the probe pulse via random phase jumps of 0-to-2\u03c0 radians every 1 cm\u22121 . b, time domain representation of the decaying molecular vibrations (upper black), incoherent probe pulse train obtained by applying the spectral phase noise to the broadband probe (middle green), and the resulting anti-Stokes pulse train (lower red). Being a product of the vibrational amplitude and the probe \ufb01eld amplitude, the output anti-Stokes \ufb01eld acquires spectral correlations due to the periodic vibrational modulation superimposed onto the uncorrelated input noise. c, Auto-correlation of the calculated noisy anti-Stokes spectrum (shown in the inset, and exhibiting no clear evidence of the Raman modes) with a single realization of the phase noise (upper red) and after averaging over 100 noise realizations (lower blue). The strong peak at 27 cm\u22121 and weak peak at 218 cm\u22121 , marked by the dotted lines, correspond to the beating of the vibrational modes of Toluene at 782, 1000 and 1027 cm\u22121 . 108 \f2.2. Method Content is comparable with the decay time of the vibrational coherence. We \ufb01rst demonstrate the new method by implementing it in a typical multi-color noncollinear boxcars geometry[3] (see Fig. 2.2.1b(i)). The setup consisted of a commercial Ti-Sapphire regenerative ampli\ufb01er providing the probe pulses at a central wavelength of 800nm, and an optical parametric ampli\ufb01er generating the pump and Stokes pulses at 1111 nm and 1250nm, respectively. All three pulses were focused into a quartz cuvette containing a liquid mixture of Toluene with ortho-Xylene (see Methods for details). The anti-Stokes spectrum was measured with a CCD-based spectrometer, while the noise was introduced by means of a home made programmable spectral pulse shaper. The auto-correlation spectrum presented in Fig. 2.7a was averaged over 100 realizations of noise. Well resolved side-bands at \u00b127 cm\u22121 and \u00b149 cm\u22121 in Fig. a correspond to the beating frequencies between the strongest excited vibrational modes of the mixed sample. In agreement with our theoretical treatment and numerical simulations, the best performance of NASCARS is obtained with a maximum (2\u03c0 peak-to-peak) phase modulation, while the spectral resolution can be controlled through the pulse shaper by varying the distance between the consecutive phase jumps in the pulse spectrum, \u03b4\u03c9n . An easier way of scrambling the probe phase without the shaper is shown in Fig. 2.2.1b(ii). When coupled to a standard multimode \ufb01bre, the probe pulse breaks apart into an incoherent pulse train due to the intermodal dispersion, and generates similar auto-correlation spectra. Numerous applications in vibrational spectroscopy, microscopy and imaging call for a single-pulse technique, recently developed by many groups[11, 12, 24, 25] and based on covering the pump, Stokes and probe wavelengths with a broad spectrum of a single ultrashort pulse. Here we demonstrate a single-pulse NASCARS measurement, based on the following mechanism. If the applied noise introduces only partial de-coherence of the original pulse, the remaining coherent part executes an impulsive pump-Stokes excitation, while the incoherent noisy part of the pulse serves as a probe. To NASCARS advantage, such partial de-coherence can be imposed on a laser beam without an elaborate shaping technology, which typically requires delicate optical alignment, calibration, maintenance, and costly optical components. We 109 \f2.2. Method Content a b Amplitude (a.u.) a 0 730 0 50 100 740 \u021c (nm) 150 200 Frequency (cm-1) 150 750 250 47 0 50 100 250 173 126 350 Frequency (cm-1) 150 200 450 250 300 Frequency (cm-1) Figure 2.7: Experimental NASCARS spectra (solid) compared with the auto-correlation of the spontaneous Raman spectra obtained by the commercial Raman spectrometer (dashed). a, Mixture of Toluene and orthoXylene with the relevant Raman shifts of 782, 1000, 1027, 982 and 1049 cm\u22121 . Dotted lines point to the strong beating signals at 27, 49 and 218 cm\u22121 . The uncorrelated spectral phase noise was introduced to the probe \ufb01eld through the pulse shaper (Fig. 2.2.1b (i)). Anti-Stokes spectrum for a single noise realization is shown in the inset. The observed linewidth is determined by the convolution of the real resonance width of \u223c3 cm\u22121 and the spectral resolution of the pulse shaper (\u223c3.5 cm\u22121 ) which determines the correlation length of the applied spectral noise. b, Single-pulse NASCARS results for the sample of liquid CBrCl3 . Here, a single ultrashort pulse was focused directly in the medium. A thin sheet of a scattering material was placed inside the compressor stage of the laser system (Fig. 2.2.1b (iii)) to create partial de-coherence of the beam. Vibrational beating at 47, 126 and 173 cm\u22121 is clearly identi\ufb01able at the expected locations (dotted lines). The observed peaks are associated with the three Raman modes of CBrCl3 at 246, 293 and 419 cm\u22121 , shown on the spontaneous Raman spectrum in the inset. 110 \f2.2. Method Content implemented a single-pulse NASCARS by simply introducing a light scatterer inside the pulse compressor of our laser system (see Fig. 2.2.1b(iii)) and Methods section for details). Placed in the way of a spectrally dispersed beam, the scattering element - a single sheet of a standard lens paper - transmits only some frequency components of the pulse while blocking the others. Standard pulse characterization shows that in accord with the aforementioned requirement, the output laser pulse consists of an ultrashort coherent part and a long noisy tail. Statistical averaging over the realizations of noise is performed by moving the scatterer between the consecutive readouts of the anti-Stokes spectrum. The resulting auto-correlation spectrum of CBrCl3 , shown in Fig. 2.7b, exhibits three clearly resolved peaks at the expected beating frequencies of the molecule, attesting to the feasibility of the proposed method. Remarkably, the whole setup consists of a single slightly modi\ufb01ed light source and a spectrometer, yet the achieved resolution of 20 cm\u22121 surpasses the spectral bandwidth of our pulses (> 500 cm\u22121 ) by more than an order of magnitude. The demonstrated implementation simplicity of noise auto-correlation spectroscopy with broadband pulses positions it as a powerful tool for chemical analysis. In all practical cases, the retrieved auto-correlation of the vibrational spectrum retains the uniqueness of the spectrum itself, and can therefore be used as an excellent \ufb01ngerprint for molecular identi\ufb01cation. As the average di\ufb00erence between the beating frequencies is usually smaller than the average frequency of vibration, the resolving power of NASCARS is lower than that of traditional CARS and may limit its application to relatively simple molecular systems. With no stringent requirements on the quality of the excitation pulse(s), the method may prove especially valuable for the applications in nonlinear microscopy by allowing the delivery of the pulses through the standard high-core-area multi-mode optical \ufb01bre, normally prohibited due to the intermodal \ufb01bre dispersion. In contrast to multiplex CARS, the pump, Stokes and probe pulses in NASCARS are all spectrally broad. As a result, the distribution of the available laser power between these components is independent of the desired spectral resolution and can therefore be adjusted for better performance, e.g. by varying the 111 \f2.2. Method Content applied noise level. By the very nature of random noise, the required averaging can be performed in a quick and robust way. Utilizing pseudo-random phase masks, specially designed for the low correlation background, may further reduce the required amount of averaging. In principle, simultaneous detection of multiple anti-Stokes spectra, observed at di\ufb00erent scattering angles and, therefore, corresponding to di\ufb00erent noise realizations, should enable a single-shot NASCARS measurement. 2.2.2 Methods The experiments in the multi-color non-collinear geometry (Fig. 2.2.1b(i,ii)) were carried out in a typical CARS setup which consists of a commercial TiSapphire regenerative ampli\ufb01er (Spit\ufb01re, Spectra-Physics, 1 KHz repetition rate, 10 nm spectral bandwidth (fwhm), 2 mJ output pulse power) generating the probe pulses at the central wavelength of 800nm, and an optical parametric ampli\ufb01er (TOPAS, Light Conversion) generating the pump and Stokes pulses at 1111 nm and 1250nm, respectively. All three pulses of \u223c10 \u03bcJ energy each were focused by a lens (focal length of 500 mm) into a quartz cuvette (5 mm optical path) with the liquid sample, where they overlapped in time and in space (BOXCARS phase-matching geometry). The output anti-Stokes beam was collimated with a 150 mm focal-length lens and coupled into the spectrometer (model 2035, McPhearson) equipped with a CCD camera (iDus DV400, Andor) and providing a spectral resolution of < 2 cm\u22121 . In the \ufb01rst con\ufb01guration (Fig. 2.2.1b(i)), we introduced white noise in the probe pulses using the programmable spectral pulse shaper based on a dual-mask 128-pixel liquid-crystal spatial light modulator (SLM-128, CRI). The resolving power of the shaper was \u223c3.5 cm\u22121 per pixel, which dictated the smallest frequency correlation length of the applied noise, and therefore determined the spectra resolution of the NASCARS signal. From studying the e\ufb00ects of the phase and amplitude noise independently, we conclude that the phase noise results in superior NASCARS performance. In contrast to the amplitude noise, it does not attenuate the available probe pulse energy 112 \f2.2. Method Content and results in a much smaller temporal overlap of the probe train with the pump-Stokes pulse pair, reducing the non-resonant background and increasing the signal quality. We also demonstrated one simple way of phase scrambling by replacing the pulse shaper with a 3 meters-long piece of a standard multi-mode \ufb01bre of 64 \u03bcm core diameter (Fig. 2.2.1b(ii)). A probe pulse, coupled into the multiple \ufb01bre modes, breaks apart into an incoherent pulse train due to the intermodal dispersion. The large number of the available modes and the high sensitivity of the dispersion of each mode to local mechanical stresses in the \ufb01bre, enables an easy and e\ufb03cient way of statistical averaging over the realizations of noise. New realizations of a random probe train are generated by simply moving the \ufb01bre between the consecutive data acquisitions. Matching the temporal duration of the output random train to the decay time of the vibrational coherence by choosing an optimal \ufb01bre length assures high spectral resolution of the NASCARS measurement. For the single-pulse experiments we used ultrashort pulses of higher bandwidth from a di\ufb00erent femtosecond Ti:Sapphire regenerative ampli\ufb01er system (Spit\ufb01re Pro, Spectra-Physics, 1 KHz repetition rate, 35 nm spectral bandwidth (fwhm), 3 mJ output pulse power). The wavelength of the ampli\ufb01ed pulses was centered at 805 nm. The beam was apertured down to the diameter of 0.5 mm before entering the compressor stage of Spit\ufb01re Pro. A thin sheet of a light scattering material (optical cleaning tissue, Thorlabs) was \ufb01xed on a rigid frame and mounted on a one-dimensional translation stage inside the compressor (Fig. 2.2.1b(iii)). The scatterer was placed after the second re\ufb02ection from the di\ufb00raction grating, i.e. at the location where all spectral components of the pulse are parallel and spatially separated. Di\ufb00erent noise realizations in this single-pulse con\ufb01guration were achieved by moving the scattering sheet perpendicular to the dispersed beam. The energy of the output beam was 10 \u03bcJ. A long-wave pass \ufb01lter (LWP) (LP02785RU-25, Semrock, cuto\ufb00 wavelength of 785nm) was used to block the high frequency components of the beam in front of the sample. The laser beam was focused into a quartz cuvette with a liquid sample (5 mm optical path) by a spherical mirror with 300 mm focal length. The transmitted laser 113 \f2.2. Method Content beam was collimated with a lens (150 mm focal length) and, after passing a short wave pass \ufb01lter (SWP) (SP01-785RU-25, Semrock, cuto\ufb00 wavelength of 785nm), coupled into the spectrometer (model 2035, McPhearson) equipped with a CCD camera (iDus DV400, Andor). The resolving power of the spectrometer in this case was 1.3 cm\u22121 . In all our experiments, each measured anti-Stokes spectrum corresponded to a di\ufb00erent noise realization. After normalization, each two consecutive spectra were subtracted from one another to remove the non-resonant background. An auto-correlation of the di\ufb00erential spectrum represented the result of a single NASCARS measurement. The statistical averaging of the auto-correlation was performed over 100 noise realizations. 114 \fBibliography [1] D. Oron, N. Dudovich, D. Yelin, and Y. Silberberg, Physical Review Letters 88 (2002). [2] D. Pestov, R. K. Murawski, G. O. Ariunbold, X. Wang, M. C. Zhi, A. V. Sokolov, V. A. Sautenkov, Y. V. Rostovtsev, A. Dogariu, Y. Huang, et al., Science 316, 265 (2007). [3] A. M. Zheltikov, Journal of Raman Spectroscopy 31, 653 (2000). [4] J. X. Cheng and X. S. Xie, Journal of Physical Chemistry B 108, 827 (2004). [5] M. O. Scully, G. W. Kattawar, R. P. Lucht, T. Opatrny, H. Pillo\ufb00, A. Rebane, A. V. Sokolov, and M. S. Zubairy, Proceedings of the National Academy of Sciences of the United States of America 99, 10994 (2002). [6] C. H. R. Ooi, G. Beadie, G. W. Kattawar, J. F. Reintjes, Y. Rostovtsev, M. S. Zubairy, and M. O. Scully, Physical Review A 72 (2005). [7] J. X. Cheng, A. Volkmer, L. D. Book, and X. S. Xie, Journal of Physical Chemistry B 106, 8493 (2002). [8] M. Schmitt, G. Knopp, A. Materny, and W. Kiefer, Chemical Physics Letters 270, 9 (1997). [9] T. Lang, K. L. Kompa, and M. 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Albrecht, Chemical Physics Letters 263, 185 (1996). [21] M. J. Stimson, D. J. Ulness, and A. C. Albrecht, Journal of Raman Spectroscopy 28, 579 (1997). [22] O. Kinrot, I. S. Averbukh, and Y. Prior, Physical Review Letters 75, 3822 (1995). [23] I. S. Averbukh, M. Shapiro, C. Leichtle, and W. P. Schleich, Physical Review A 59, 2163 (1999). [24] B. von Vacano, W. Wohlleben, and M. Motzkus, Journal of Raman Spectroscopy 37, 404 (2006). [25] Y. Paskover, I. S. Averbukh, and Y. Prior, Optics Express 15, 1700 (2007). 116 \fChapter 3 Narrowband Spectroscopy by All-optical Correlation of Broadband Pulses 3.1 Motivation In Chapter 2, the method of noise auto-correlation spectroscopy with coherent raman scattering (NASCARS) was introduced. NASCARS can extract the vibrational level spacing through autocorrelations of CARS spectra. The single pulse version of NASCARS method can be performed on a simple experiment setup without a pulse shaper. However, the limitation of NASCARS is obvious: the autocorrelation of the vibrational spectrum is not equivalent to the spectrum itself. It does not re\ufb02ect absolute locations of the resonances, and the linewidth of the autocorrelation spectrum is often broader than that of the spectrum. In this chapter, the method of narrowband spectroscopy by all-optical correlation of broadband pulses is introduced to give the absolute location of the vibrational levels. This method is based on a cross-correlation optical processing between the CARS signal and a reference pulse of broad bandwidth. The cross-correlation optical processing is related to sum frequency generation between the CARS \ufb01eld ECARS (t) and a reference \ufb01eld Eref (t). The cross-correlation \ufb01eld ESF G (t) is proportional to the product of the CARS 0 A version of this chapter is in-press as Stanislav O. Konorov, Xiaoji G. Xu, John. W. Hepburn and Valery Milner \u201cNarrowband Spectroscopy by All-optical Correlation of Broadband Pulses\u201d, in Physical Review A 117 \f3.1. Motivation \ufb01eld and the reference \ufb01eld ESF G (t) \u221d ECARS (t) \u00b7 Eref (t) (3.1) The CARS \ufb01eld ECARS (t) is proportional to the product between the vibrational coherence R(t) and the probe pulse \ufb01eld Epr (t) ECARS (t) \u221d Epr (t) \u00b7 R(t) (3.2) One can combine expressions (3.1) and (3.2), and the order of multiplication can be regrouped into: ESF G (t) = R(t) \u00b7 [Epr (t) \u00b7 Eref (t)] (3.3) The time domain spectrum of the cross-correlation signal is obtained through Fourier transform. ESF G (\u03c9) = R(\u03a9) \u2297 f f t{[Epr (t) \u00b7 Eref (t)]}[\u03c9] (3.4) Following the same line of reasoning as in section 5.1, the e\ufb03ciency of the information transfer from the vibrational coherence R(t) is a\ufb00ected by the temporal shape of [Epr (t) \u00b7 Eref (t)]. The desirable pulse product [Epr (t) \u00b7 Eref (t)] in the time domain should have a long duration so as to overlap with the duration of R(t). In the frequency domain, the Fourier transform of pulse pairs [Epr (t)\u00b7Eref (t)] should give a narrow band frequency component. In this chapter, two broad band pulses E1 and E2 that can generate a sum-frequency spectrum with only one narrow band frequency component is de\ufb01ned as a conjugate pulse pair. The ideal mathematical de\ufb01nition is \u03b4(\u03c9) \u2261 E1 (\u03c9) \u2297 E2 (\u03c9). A simple realization of such a conjugate pair can be found by creating chirped pulses. If the probe pulse and reference pulse contains the same amount of chirp but with opposite sign, the products of [Epr (t) \u00b7 Eref (t)] will show long time duration and a narrow frequency bandwidth in the frequency domain. Experimentally, one pulse from a conjugate pair is used 118 \f3.1. Motivation as a probe pulse, then other pulse can be used to perform sum frequency generation with the CARS \ufb01eld and the sum frequency spectrum should re\ufb02ect the pro\ufb01le of the vibrational coherence R(\u03a9). Because creating such a conjugate pulse pair needs two pulse shapers, which inevitably increases experimental complexity, a further investigation was made to \ufb01nd a self-conjugate pulse i.e. [Epr (t) \u2261 Eref (t)]. Such a pulse 2 (t) and a should satisfy the requirement of having a long duration of Epr narrow bandwidth in the second harmonic spectrum. The self-conjugate pulse is used as both the probe pulse in the CARS generation and the reference pulse in the sum frequency generation. One type of spectral phase pattern that is particularly useful on generating a narrow band second harmonic spectrum is the anti-symmetric spectral phase: \u03c6(\u03c9c + \u0394) = \u2212\u03c6(\u03c9c \u2212 \u0394) (3.5) with \u03c9c being the pulse center. Such pulse shapes has been systematically studied by Dantus and coworkers [1, 2]. The generation of narrow band frequency component of Epr (t) \u00b7 Epr (t) in the frequency domain can be understood by the following derivation. The frequency domain spectrum of the \ufb01eld product Epr (t) \u00b7 Epr (t) is equivalent to the second harmonic generation expression (3.6) ESHG (\u03c9) = \u0003 \u221e \u2212\u221e Epr (\u03a9)Epr (\u03c9 \u2212 \u03a9)d\u03a9 (3.6) The spectrum of ESHG at the frequency of 2\u03c9 is ESHG (2\u03c9) = \u0003 \u221e \u2212\u221e |Epr (\u03a9)| \u00b7 |Epr (2\u03c9 \u2212 \u03a9)|ei\u03a6 d\u03a9 (3.7) with ei\u03a6 as the phase term, it is the sum of spectral phase \u03a6(2\u03c9) = \u03c6(\u03a9) + \u03c6(2\u03c9 \u2212 \u03a9). With the condition that the spectral phase of the probe pulse satis\ufb01es \u03c6(\u03c9c + \u03b4) = \u2212\u03c6(\u03c9c \u2212 \u03b4) for all \u0394, it is not hard to \ufb01nd that the phase term \u03a6 = 0 when \u03c9 = \u03c9c and \u0394 = \u03a9 \u2212 \u03c9c . With the spectral phase term \u03a6 equal to zero at the center of SFG spectrum 2\u03c9c , the integral of the expression (3.7) reaches its maximal value, giving a peak in the spectrum. 119 \f3.1. Motivation The anti-symmetric spectral phase pattern provides a peak at twice the central frequency. However, having the anti-symmetric spectral phase pattern is not the only requirement for the self-conjugate pulse. A pulse that has anti-symmetric spectral phase pattern can also have other frequency components in the second harmonic spectrum. An extreme case is the transform-limited pulse. With the spectral phase equals zero, the transform-limited pulse trivially satis\ufb01es the requirement set by expression (3.5). But the second harmonic spectrum of the transform-limited pulse has a broad peak rather than a narrow peak. To further narrow down the peak of the second harmonic, the spectral phase modulation based on noise was investigated. When the uncorrelated high amplitude spectral noise is introduced into the pulse in addition to the anti-symmetric spectral phase requirement, the second harmonic spectrum is narrowed. However, due to the \ufb01nite pixel number of the pulse shaper, even with the anti-symmetry spectral phase restriction, random noise patterns often create residual peaks beside the central peak in the second harmonic spectrum. To remove the residual peaks in the second harmonic spectrum, the genetic algorithm optimization was further used. The genetic algorithm (GA) has been used in many applications in chemical physics[3, 4]. It uses the experiment or process output as a \ufb01tness value, optimizing input parameter sets to \ufb01nd the best \ufb01tness value through hybridization of multiple best parameter sets. With the utilization of the pulse shaper, the spectral phase of a broad band pulse can be used as input parameters, and GA can search the best available phase pattern to ful\ufb01ll a given task. The optimization on the narrow central peak in the second harmonic spectrum can then be addressed through a GA optimization. The experiment started with the measurement of the probe pulse spectrum. Then, a computer-run GA optimization searching for the good quality self-conjugate probe pulse was carried out. Then the pulse shaper tailored the phase shape of the probe pulse according to the GA output. The CARS signal was generated by pump\/Stokes and probe pulses and collimated to generate the sum frequency signal in a nonlinear crystal. As the article section shows, the sum frequency spectrum showed the exact spectrum of the 120 \f3.2. Experimental Technique Considerations vibrational coherence R(\u03a9). The method of \u201cnarrowband spectroscopy by all-optical correlation of broadband pulses\u201d can achieve a good resolution vibrational spectrum while using all broad band pulses. Comparing to NASCARS, the method gives the spectrum of the vibrational resonances rather than the autocorrelation of the spectrum. The resolution of this method is limited by the bandwidth of the central peak in the second harmonic spectrum of the optimized selfconjugate probe pulse. It is not limited by the broad bandwidth of the probe pulse. However, this method requires additional experiment instruments on generating the SFG signal when compared to a typical multiplex CARS setup. The current intensity of the generated SFG signal is lower than the direct CARS signal by two orders of magnitude, which is due to the low conversion e\ufb03ciency of the nonlinear crystal. With better non-linear crystal, the signal strength can be further improved. 3.2 Experimental Technique Considerations In addition to a typical BOXCARS geometry CARS setup (\ufb01gure 1.23), the optical processing of CARS requires additional experimental setup for sum frequency generation. The generated CARS signal has to be mixed with the reference pulse in a nonlinear crystal. Nonlinear mixing is usually done with high intensity pulses. Due to the weak intensity of CARS signal, it requires careful work to achieve the spatial overlapping between CARS signal and the reference probe pulse. The spatial overlapping of weak pulses was facilitated by using a small pin hole mounted on a two dimensional adjustable translation stages. Excitation pulses were adjusted to pass through the pin hole. A typical surveillance camera behind the pin hole was used to monitor the laser beam position. The thickness of the nonlinear crystal is also a concern for the intensity of the SFG signal. The choice is primarily between the e\ufb03ciency and distortion. Thicker crystals give higher conversion e\ufb03ciency, but are more limited in phase matching conditions than thinner crystals. Both 30\u03bcm and 100\u03bcm type-I BBO crystal were used in the experiment. The thin 30\u03bcm crystal is 121 \f3.3. Method Content insensitive to crystal angle on sum frequency generation but gives low signal strength due to a short interaction length. The 100\u03bcm type-1 BBO gives good conversion e\ufb03ciency but require adjustment on the crystal orientation. In the experiment demonstration, the 100\u03bcm crystal was used. The detailed calculation can be carried use the equation (1.51) in section 1.3. To reduce the dispersion that comes from light passing through lenses, mirrors were used as the collimating and focusing element in the CARS generation and sum frequency generation. To compensate the group velocity dispersion, the beam-split reference probe pulse went through an identical sample cell. The dispersion compensation techniques was found to be able to improve signal to noise ratio for the \ufb01nal sum-frequency spectrum. 3.3 3.3.1 Method Content Overview High peak power ultrafast lasers are widely used in nonlinear spectroscopy but often limit its spectral resolution because of the broad frequency bandwidth of ultrashort laser pulses. Improving the resolution by achieving spectrally narrow excitation of, or emission from, the resonant medium by means of multi-photon interferences has been the focus of many recent developments in ultrafast spectroscopy. We demonstrate an alternative approach, in which high resolution is exercised by detecting narrow spectral correlations between broadband excitation and emission optical \ufb01elds. All-optical correlation analysis, easily incorporated into the traditional spectroscopic setup, enables direct, robust and simultaneous detection of multiple narrow resonances with a single femtosecond pulse. 3.3.2 Content With recent advances of ultrafast laser sources, featuring high optical \ufb01eld amplitudes at low average power, coherent nonlinear spectroscopy with femtosecond (fs) pulses has been recognized as a promising tool for time-resolved chemical analysis [5\u20137], remote sensing of complex molecules [8, 9] and non122 \f3.3. Method Content invasive imaging of biological objects [10\u201312]. Due to the broad spectral width of ultrashort pulses, femtosecond spectroscopy often lacks spectral resolution. The latter can be recovered by complementing the frequency resolved measurement with the time-delay scanning [13, 14], or by combining the broadband fs excitation with the narrowband probing by picosecond pulses from a separate laser source [15] or a spectral slice of a femtosecond source [16, 17] (\u201cmultiplex cars\u201d). Alternatively, higher resolution can also be achieved without resorting to narrowband pulses and without the time-consuming delay scans. As many nonlinear optical methods involve interferences between multiple photons of di\ufb00erent frequencies from under the same pulse bandwidth, improving the resolution is possible by controlling these interferences with spectral pulse shaping [18]. Spectral resolution, signi\ufb01cantly better than the broad bandwidth of ultrashort laser pulses, has been achieved in second harmonic generation [19], multi-photon absorption [1, 20, 21] and coherent Raman scattering [22, 23] of shaped femtosecond pulses. In this work we focus on Coherent Anti-Stokes Raman Scattering (cars) which has become a popular method in nonlinear optical spectroscopy and microscopy because of its high sensitivity to molecular structure [24]. In cars, two laser photons, \u201cpump\u201d and \u201cStokes\u201d, excite the coherent molecular vibrations, which then scatter a third, \u201cprobe\u201d, photon generating the anti-Stokes signal. Despite the broad spectrum of the femtosecond pump and Stokes pulses, their collective two-photon \ufb01eld can be spectrally narrowed by means of the pulse chirping [25] or shaping [22], providing selectivity of Raman excitation. On the other hand, shaping of the probe pulse have been used for narrowing the spectrum of the anti-Stokes emission [23]. In both cases, the spectral line narrowing is a result of a delicate interference of the input \ufb01elds inside the Raman medium. As such, it is sensitive to the proper choice of the pulse shapes, non-resonant background and interferometrically stable time delays. In the recently demonstrated method of noise-autocorrelation spectroscopy [26], we have eliminated the requirement of an accurate pulse shaping, while achieving high spectral resolution without delay scanning and bandwidth 123 \f3.3. Method Content multiplexing. The method is based on the detection of optical \ufb01eld correlations in the coherently scattered light. The correlations are induced by the vibrational resonances, and therefore carry the information about the Raman spectrum of the medium. The auto-correlation of the Raman spectrum has been extracted via computer post-processing of the measured data, which involved numerical correlation analysis with averaging over multiple noise realizations. Here, we show that spectral correlations in the coherently scattered broadband anti-Stokes radiation can produce a narrowband optical Raman spectrum similar to that obtained with spontaneous Raman or multiplex cars, yet without the narrowing of the pulse bandwidth. We take advantage of the possibility to detect optical correlations between two broadband pulses by means of the non-resonant interferences in the sum-frequency generation (sfg) of those pulses in the external nonlinear crystal [27]. We start with the two pulses (hereafter called \u201cconjugate\u201d probe, Epr , and reference, Eref ) designed to exhibit narrow single-peak sfg spectrum, \u0012\u0003 \u00122 \u0012 \u0012 \u0012 Epr+ref (\u03a9) \u221d \u0012 Epr (\u03c9)Eref (\u03a9 \u2212 \u03c9)d\u03c9 \u0012\u0012 \u221d \u03b4(\u03a9 \u2212 \u03c9c ), (3.8) where \u03b4 is the Dirac \u03b4-function and \u03c9c represents the central frequency of the probe\/reference sfg spectrum. The probe pulse is then scattered o\ufb00 the molecular vibrations, generating the anti-Stokes pulse. Finally, the resonance-induced correlations in the anti-Stokes light are optically processed by mixing the cars signal with the reference pulse. The measured \u000e cars\/reference sfg spectrum, Icars+ref (\u03a9) \u221d | Ecars (\u03c9)Eref (\u03a9 \u2212 \u03c9)d\u03c9|2 , re\ufb02ects the narrow vibrational modes of the medium as described below. In cars, coherent molecular vibrations are excited by a two-photon \ufb01eld of the simultaneously applied transform-limited pump and Stokes pulses, Ep and ES , respectively (black lines in Fig.3.1(a)). The induced vibrational coherence can be expressed as a product of the excitation spectrum and the spectrum of the Raman modes [14]: R(\u03a9) = A(\u03a9) \u00d7 \u0013\u0002 \u0014 k Ck (\u03a9) + Cnr , (3.9) 124 \f3.3. Method Content (b) frequency Ref SFG (a) Stokes CARS Probe Pump Figure 3.1: (Color online) (a) Schematic representation of the coherent antiStokes scattering of the spectrally shaped probe pulse (red) o\ufb00 the molecular vibrations at \u03a91 and \u03a92 , induced by the transform-limited pump and Stokes pulses (black). (b) an all-optical retrieval of the narrowband Raman spectrum by means of the sum-frequency mixing of cars and reference pulses in a separate nonlinear crystal. In this work, reference pulse is a replica of the probe pulse, spectrally shaped by means of the liquid crystal based pulse shaper (inset). 125 \f3.3. Method Content where A(\u03a9) = \u000e Ep (\u03c9)ES (\u03a9 \u2212 \u03c9)d\u03c9, Ck (\u03a9) represents the contribution of the nth resonance, and the non-resonant background is denoted Cnr . AntiStokes scattering of the probe \ufb01eld, Epr , o\ufb00 the molecular vibrations results in the cars signal, Ecars , which in the time domain can be written as: Ecars (t) \u221d R(t)Epr (t), (3.10) with R(t) being the Fourier transform of the spectral response, R(\u03a9). The sum-frequency generation \ufb01eld of the cars and reference pulses is, therefore: Ecars+ref (t) \u221d Ecars (t)Eref (t) = Epr (t)Eref (t)R(t), (3.11) which in the frequency domain corresponds to the convolution of the probe\/reference sfg spectrum, Epr+ref (\u03c9), and the vibrational spectrum of the medium: \u0003 Ecars+ref (\u03c9c + \u03a9) = Epr+ref (\u03c9c \u2212 \u0394)R(\u03a9 + \u0394)d\u0394. (3.12) Thus, by narrowing the spectrum of Epr+ref (Eq.3.8), one can establish an exact correspondence between Ecars+ref (\u03c9c + \u03a9) and R(\u03a9), retrieving the Raman frequency shifts directly from the measured sfg signal. Unlike the all-optical processing used in multiplex cars and based on the resonant interference between the excited vibrational states and their precise amplitude and phase shaping [28], our approach does not require any prior knowledge on the vibrational frequencies of the molecules. It is also not sensitive to the particular spectral shape of the probe pulses as long as the conjugation condition of Eq.3.8 is satis\ufb01ed. The conjugate probe and reference pulses can be generated by various means, including simple frequency chirping or frequency down conversion [29]. Here, we employ spectral pulse shaping to create a \u201cself-conjugate\u201d pulse, i.e. a broadband pulse with a narrowband second harmonic, Epr+ref (\u03a9) \u2192 Epr+pr (\u03a9). The self-conjugate \ufb01eld serves both as the probe and the reference, thus eliminating the need of dealing with two separate pulses and simplifying the experimental setup. This result, shown schematically in Fig.3.1(b), provides the basis for the experimental method demonstrated in this work. 126 \f3.3. Method Content Intensity (arb.units) 1 (a) (b) (c) (d) .8 .6 .4 .2 Intensity (arb.units) 0 .8 .6 .4 .2 0 700 800 900 1000 1100 1200 1300 Raman shift (cm-1) -300 -200 -100 0 100 200 300 Frequency (cm-1) Figure 3.2: (Color online) Numerical simulations of the proposed method. (a) Model spectrum of a toluene\/orto-xylene mixture. (b) Calculated cars spectrum for the case of a pseudo-randomly shaped probe (see text). (c,d) Calculated spectra of the cars\/probe sfg and probe shg signals, respectively, for the case of the non-optimized (green) and optimized (red) pseudorandom probe shaping. The line width is de\ufb01ned by the frequency resolution of the model pulse shaper (4.7 cm\u22121 ), rather than by the overall bandwidth of the probe pulse (dashed lines). 127 \f3.3. Method Content Self-conjugate pulses can be generated by shaping the original transformlimited femtosecond pulse with a pseudo-random binary phase mask [30]. As a two-photon process, second harmonic generation (shg) at any given frequency \u03c9c is de\ufb01ned by the interference of multiple photon pairs, whose total frequency adds up to \u03c9c . For this to result in a narrowband spectrum, the interference must be constructive at \u03c9c and destructive everywhere else. The \ufb01rst requirement is known to be satis\ufb01ed by the condition \u2217 (\u03c9 \/2 + \u0394) [20], which can be realized by applying an Epr (\u03c9c \/2 \u2212 \u0394) = Epr c anti-symmetric spectral phase shaping around \u03c9c \/2. Destructive interference can be achieved by randomizing the spectral phase of the pulse while preserving the anti-symmetric property [30, 31]. Calculations of the sum-frequency mixing of the probe and cars pulses (Eq.3.12), and its correspondence to the model vibrational spectrum of the medium, are shown in Fig.3.2(a,c). First, an uncorrelated white noise, antisymmetrized around the central frequency, has been added to the phase of the originally transform-limited probe \ufb01eld through a model pulse shaper. Owing to the presence of Raman resonances and despite the uncorrelated noise in the probe, spectral correlations are created in the cars \ufb01eld. Though not apparent in the cars signal itself (Fig.3.2(b)), they produce sharp peaks in the cars\/probe sfg spectrum (Fig.3.2(c)), which can be clearly assigned to the corresponding Raman lines. Unfortunately, residual correlations in the random phase give rise to the arti\ufb01cial lines and lower signal-to-noise ratio, seen both in the cars\/probe sfg and probe\/probe shg spectra (Fig.3.2(c) and (d),respectively). To improve the quality of the signal, we performed a numerical optimization based on the genetic algorithm search of a pseudo-random binary phase mask (constrained to 0 and \u03c0 radian only [30]) resulting in the narrowest calculated probe shg spectrum. Due to the \ufb01nite spectral resolution of the pulse shaper and, therefore, \ufb01nite width of the optimized shg, the correspondence between Ecars+pr (\u03c9c + \u03a9) and R(\u03a9) in Eq.3.12 is not exact. Hence, using the cars\/probe sfg line width as a \ufb01tness parameter improved the performance of the method even further, but required a priori assumption about the line width of the Raman resonances. The resulting pseudo-random bi128 \f3.3. Method Content nary masks were used in the experiments described below. The experimental setup (Fig.3.3) was based on a standard Ti:Sapphire regenerative ampli\ufb01er, producing 40 fs probe pulses at the central wavelength of 800 nm and 1 KHz repetition rate. An optical parametric ampli\ufb01er generated the pump and Stokes beams at 1111 and 1250 nm, respectively. Pre-calculated spectral phase has been applied to the probe pulses by means of a home-made pulse shaper based on a liquid-crystal spatial light modulator (see inset in Fig.3.1) and provided spectral resolution of 10 cm\u22121 . Pump, Stokes and probe pulses, about 2 \u03bcJ each, have been focused by a silver coated mirror into a quartz cuvette with liquid toluene, where they overlapped in time and space in the standard boxcars phase-matching geometry. cars signal has been then collimated and focused onto a 100 \u03bcm BBO crystal, together with the reference pulse which has been split o\ufb00 the shaped probe pulse in front of the sample. Sum-frequency signal from the nonlinear mixing of the cars and reference pulses has been coupled into a high-resolution spectrometer equipped with a CCD camera, and typically accumulated for about 1 minute. Experimental sfg spectra are presented in Fig.3.4(a). The spontaneous Raman spectrum of toluene, measured separately, is shown at the top of the plot for reference. Below it, the two signals with sharp peaks of much narrower width than the bandwidth of the probe pulse, attest to the high resolution of the proposed method. The position of the two peaks of the center curve match the frequencies of the two strong Raman modes of toluene around 1000 and 784 cm\u22121 , covered by the broad bandwidth of the pump\/Stokes pulse pair. The latter is demonstrated by the observed cars signal, with and without phase shaping, in plot (b). The apparently random cars intensity distribution in the shaped case results from the presence of Raman modes and carries the information about their frequencies, which is revealed in the cars\/probe sfg spectrum. The sfg spectrum at the bottom of Fig.3.4(a) exhibits low signal-to-noise ratio as a result of the lack of the phase mask optimization. An optimized mask has resulted in higher quality spectrum shown in the middle of the plot. Note that the optimization has not been performed during the experiment 129 \f3.3. Method Content CARS NLC M2 Probe spectrometer CCD Sample DL Probe optical shaper Ti:Sapphire laser Pump S M1 Stokes OPA DL DL Figure 3.3: Experimental setup. Transform-limited pump and Stokes pulses from an optical parametric ampli\ufb01er (OPA) and a shaped probe pulse from the pulse shaper are focused on a 5 mm thick sample by a 20 cm focal length mirror (M1 ). Output cars pulse is then focused by a similar mirror (M2 ) on a nonlinear crystal (NLC), together with a replica of the probe pulse, to produce a sum-frequency generation signal, which is detected by a spectrometer (spectral resolution of 0.05 nm). The probe beam, used as a reference, is passed through an identical sample cuvette (S) to compensate the accumulated dispersion of the cars signal. DL - delay lines. 130 \f3.3. Method Content Raman shift, \u0226 (cm-1) 1200 900 Frequency, \u0226 (cm-1) 600 1500 (a) 3.0 1200 900 600 CARS 300 (b) Intensity (arb.units) 2.5 2.0 SFG \u021c = 720 740 300 0 \u0226 = 600 1.5 760 -300 SHG 780 -600 (c) 1.0 0.5 0.0 380 385 390 Wavelength, \u021c (nm) 395 390 400 Wavelength, \u021c (nm) 410 Figure 3.4: (Color online) (a) Experimentally observed cars\/probe sfg spectra (middle and bottom) in comparison to the spectrum of spontaneous Raman scattering (top). Black, green and red curves correspond to the case of unshaped, non-optimized shaped and optimized shaped probe pulse, respectively. (b) cars spectra for the shaped (red) and unshaped (black) probe pulses. (c) The spectra of the second harmonic of the shaped (red) and unshaped (black) probe pulses. 131 \f3.3. Method Content in an adaptive feedback-controlled fashion, in which the observed spectral contrast would have been used as a \ufb01tness parameter. Instead, we have pre-calculated our binary phase masks for the anticipated resonance line width and the measured characteristics of the probe pulse (i.e. its spectral intensity and phase before shaping). The latter proves critical for the quality of the observed sfg signal. We therefore attribute the unequal performance of di\ufb00erent masks to the uncertainty in characterizing the probe pulse, which will be improved in the future. As expected, spectral narrowing of the cars\/probe sfg signal is accompanied by the corresponding narrowing of the probe\u2019s second harmonic, shown in Fig.3.4(c). We have found that for our experimental parameters, better peak-to-background contrast in the sfg always corresponds to the better contrast of the shg peak. The reason for this is the insu\ufb03cient resolution of our pulse shaper for resolving the line width of the observed Raman modes (10 cm\u22121 vs 3 cm\u22121 , respectively). As a result, the optimization is almost insensitive to the width of the resonant lines and works equally well for both the sfg and shg narrowing. This however, may not be true for the case of higher resolution shaping. The demonstrated approach presents an alternative to the existing methods of high-resolution Raman spectroscopy with ultrashort pulses, which typically rely on the delay scanning, interferometric stability, or post-processing of the acquired data. All-optical correlation analysis is performed separately from the resonant medium of interest, reducing the sensitivity of the method to non-resonant background, precise time delays, and other laser parameters. The ability to detect Raman peaks directly in the measured sfg spectrum may prove invaluable for the applications in microscopy. For instance, sensitive detection of the integral sfg signal, passed through an appropriate frequency \ufb01lter, could quickly identify the presence of a certain Raman mode without the need of a spectrometer. Though this type of detection is similar to the traditional spontaneous Raman or multiplex cars spectroscopy, the proposed method utilizes the whole spectral bandwidth and high peak power of femtosecond pulses, thus suggesting the possibility for higher sensitivity or faster data retrieval. In the proof-of-principle work presented here, 132 \f3.3. Method Content the speed was limited by the low e\ufb03ciency of the sum-frequency generation. This can be improved by using thicker nonlinear crystals with optimized dispersion properties, and by increasing the power of a reference pulse. Precalculated phase masks may enable selective detection of resonances with the speci\ufb01ed line width, while avoiding time consuming feedback-controlled optimization. 133 \fBibliography [1] I. Pastirk, J. M. Dela Cruz, K. A. Walowicz, V. V. Lozovoy, and M. Dantus, Optics Express 11, 1695 (2003). [2] V. V. Lozovoy, B. W. Xu, J. C. Shane, and M. Dantus, Physical Review A 74 (2006). [3] R. S. Judson and H. Rabitz, Physical Review Letters 68, 1500 (1992). [4] A. Assion, T. Baumert, M. Bergt, T. Brixner, B. Kiefer, V. Seyfried, M. Strehle, and G. Gerber, Science 282, 919 (1998). [5] T. H. Joo, M. A. Dugan, and A. C. Albrecht, Chemical Physics Letters 177, 4 (1991). [6] M. Schmitt, G. Knopp, A. Materny, and W. Kiefer, Chemical Physics Letters 270, 9 (1997). [7] T. Lang, K. L. Kompa, and M. Motzkus, Chemical Physics Letters 310, 65 (1999). [8] M. O. Scully, G. W. Kattawar, R. P. Lucht, T. Opatrny, H. Pillo\ufb00, A. Rebane, A. V. Sokolov, and M. S. Zubairy, Proceedings of the National Academy of Sciences of the United States of America 99, 10994 (2002). [9] C. H. R. Ooi, G. Beadie, G. W. Kattawar, J. F. Reintjes, Y. Rostovtsev, M. S. Zubairy, and M. O. Scully, Physical Review A 72 (2005). [10] A. Zumbusch, G. R. Holtom, and X. S. Xie, Physical Review Letters 82, 4142 (1999). [11] E. O. Potma, W. P. de Boeij, P. J. M. van Haastert, and D. A. Wiersma, Proceedings of the National Academy of Sciences of the United States of America 98, 1577 (2001). [12] J. X. Cheng and X. S. Xie, Journal of Physical Chemistry B 108, 827 (2004). 134 \fChapter 3. Bibliography [13] M. Heid, S. Schlucker, U. Schmitt, T. Chen, R. Schweitzer-Stenner, V. Engel, and W. Kiefer, Journal of Raman Spectroscopy 32, 771 (2001). [14] X. J. G. Xu, S. O. Konorov, S. Zhdanovich, J. W. Hepburn, and V. Milner, Journal of Chemical Physics 126 (2007). [15] J. X. Cheng, A. Volkmer, L. D. Book, and X. S. Xie, Journal of Physical Chemistry B 106, 8493 (2002). [16] D. Oron, N. Dudovich, and Y. Silberberg, Physical Review Letters 90 (2003). [17] S. H. Lim, A. G. Caster, and S. R. Leone, Physical Review A 72 (2005). [18] A. M. Weiner, Review of Scienti\ufb01c Instruments 71, 1929 (2000). [19] Z. Zheng and A. M. Weiner, Chemical Physics 267, 161 (2001). [20] D. Meshulach and Y. Silberberg, Nature 396, 239 (1998). [21] V. V. Lozovoy, I. Pastirk, K. A. Walowicz, and M. Dantus, Journal of Chemical Physics 118, 3187 (2003). [22] N. Dudovich, D. Oron, and Y. Silberberg, Nature 418, 512 (2002). [23] D. Oron, N. Dudovich, D. Yelin, and Y. Silberberg, Physical Review Letters 88 (2002). [24] A. M. Zheltikov, Journal of Raman Spectroscopy 31, 653 (2000). [25] E. T. J. Nibbering, D. A. Wiersma, and K. Duppen, Physical Review Letters 68, 514 (1992). [26] X. G. Xu, S. O. Konorov, J. W. Hepburn, and V. Milner, Nature Physics 4, 125 (2008). [27] J.-C. Diels and W. Rudolph, Ultrashort Laser pulse Phenomena (Academic Press, 2006), 3rd ed. [28] D. Oron, N. Dudovich, and Y. Silberberg, Physical Review A 70 (2004). [29] B. Dayan, A. Pe\u2019er, A. A. Friesem, and Y. Silberberg, Physical Review Letters 93 (2004). 135 \fChapter 3. Bibliography [30] M. Comstock, V. V. Lozovoy, I. Pastirk, and M. Dantus, Optics Express 12, 1061 (2004). [31] Z. Zheng and A. M. Weiner, Optics Letters 25, 984 (2000). 136 \fChapter 4 Complete Characterization of Molecular Vibrations using Frequency Resolved Gating 4.1 Motivation As discussed in section 1.3, the purpose of CARS is to prepare the vibrational coherence and recover its information through spectroscopic measurement. However, the vibrational coherence R(\u03a9) contains both amplitude and phase information. The traditional CARS methods described in chapter 1.2 and the methods that are presented in chapter 2 and chapter 3 cannot measure the phase of the vibrational coherence. In this chapter, the method of \u201cComplete Characterization of Molecular Vibrations using Frequency Resolved Gating\u201dis presented to experimentally retrieve the phase and amplitude information of the vibrational coherence from CARS spectra. As described in chapter 2, the method of NASCARS provides a simple way to extract the vibrational spacing of resonances through obtaining the autocorrelation of the vibrational coherence spectrum. In chapter 3, the method of narrowband spectroscopy by all-optical correlation of broadband pulses used optical processing techniques on the broad band CARS signal to 0 A version of this chapter has been published as Xiaoji G. Xu, Stanislav O. Konorov, Sergey Zhdanovich, John. W. Hepburn and Valery Milner \u201cComplete Characterization of Molecular Vibrations using Frequency Resolved Gating\u201dJournal of Chemical Physics Vol. 126 No.9, 2007 137 \f4.1. Motivation obtain the high resolution CARS spectrum. This spectrum contains more information on resonant levels than the autocorrelation of the spectrum. However, neither method can recover phase information. The phase information of the vibrational coherence re\ufb02ects the excitation conditions as well as the time domain behavior of the prepared vibrational levels. Moreover, as shown in \ufb01gure 1.10 of section 1.2, with phase information the Fourier transform directly links the complex spectrum of the vibrational coherence with the time domain beating of the vibrational coherence and vice versa. As a property of the Fourier transform, the resolution of the vibrational coherence in the frequency domain is determined by the total duration of the time domain response. The CARS signal in the frequency domain is the convolution between the probe pulse E(\u03c9) and the vibrational coherence R(\u03a9). The convolution process means that the frequency domain pro\ufb01le of the vibrational coherence is broadened by the probe pulse spectrum. To recover R(\u03a9) from the CARS spectrum, one seemingly obvious solution is to perform a reverse operation to the convolution i.e. deconvolution. However, the direct deconvolution process itself is not a mathematically easy question [1]. It requires a high signal to noise ratio spectrum and the exact form of the broadening function i.e. the probe pulse. Moreover, the convolution between R(\u03a9) and the probe pulse is done in the complex domain, but the measured CARS spectra do not contain the phase of the anti-Stokes \ufb01eld. This lack of phase information in the CARS \ufb01eld further undermines the feasibility of the direct deconvolution approach. The cross-correlation frequency resolved optical gating (XFROG) technique was invented by S. Linden et.al.[2] and is based on the pulse characterization technique of frequency resolved optical gating (FROG). It uses a well characterized reference pulse performing sum-frequency generation (SFG) or di\ufb00erence-frequency generation (DFG) with the optical pulse. The SFG or DFG spectra are recorded to form XFROG trace by scanning the time delay between the reference pulse and the unknown pulse. With complete information of the reference pulse, the XFROG algorithm then recovers the amplitude and the phase of the unknown pulses from the recorded data. 138 \f4.1. Motivation SFG B Reference Anti-Stokes Probe Stokes Pump A R(t) Figure 4.1: Figure A shows the scheme for the CARS process and \ufb01gure B shows that of SFG. The CARS process and be alteratively regarded as a generalized version of SFG between the vibrational coherence R(\u03a9) and the probe \ufb01eld. As discussed in section 1.3, the coherent scattering step of CARS can be treated as sum-frequency generation between the probe pulse and the vibrational coherence. Correspondence between CARS and SFG is shown in Figure 4.1. The reference pulse in SFG corresponds to the probe pulse in CARS, and the unknown pulse in SFG corresponds to the prepared vibrational coherence. Considering the fact that the mathematical algorithm of XFROG works with su\ufb03cient input parameters and data, there is a possibility of extending the XFROG technique to CARS for recovering the pro\ufb01le of R(\u03a9). A method for complete characterization of molecular vibration was proposed based on such reasoning. It requires the experimental characterization of the probe pulse in CARS (corresponding to the reference pulse in the XFROG technique) and scanning the time delay between the probe pulse and the pump\/Stokes pair and recording CARS spectra at di\ufb00erent time delays. These CARS spectra form a spectrogram with frequency and time delay (corresponding to the XFROG trace). After the CARS spectrogram is obtained, the XFROG algorithm is used to recover the amplitude and the phase of the vibrational coherence. 139 \f4.1. Motivation 0.9 V\u2019 Vi Intensity (AU) 0.8 0.7 0.6 g 0.5 0.4 0.3 0.2 0.1 0 -1 0 1 2 Time(ps) 3 4 Figure 4.2: The blue continuous curve shows the time beating of a system with 3 excited state levels that are equally spaced. The vibrational beating maximum can be found at 1.6ps (vertical dashed line). The red dashed curve shows the overall beating with another resonant level close to the three level system. Energy levels of the pure sample and the additional component are shown in the inset. 140 \f4.1. Motivation As the following article discusses, the XFROG retrieved vibrational coherence is independent of the properties of the probe pulse, therefore the proposed complete characterization method does not su\ufb00er from the intensity vs. resolution dilemma. The retrieved spectrum of the vibrational coherence has good spectral resolution ( 3cm\u22121 FWHM resonant peaks are clearly resolved), regardless of the broad bandwidth of the probe pulse (>200cm\u22121 ). With phase information available, the spectral resolution is determined by the scanning range of time delay. A 10ps scanning range can give 3cm\u22121 resolution. The ability to experimentally obtain the phase of vibrational excited levels is a unique feature that is associated with this approach. With the ability to recover the spectral phase, a demonstration of the ability to separate time domain vibrational beatings from chemical mixtures is also discussed. The current time-resolved CARS methods [3\u20135] that measure the beating between vibrational levels require pure samples. Additional chemical component in the sample can dramatically change the beating pro\ufb01le due to the interference between resonant levels. For chemical physics experiments that involve utilizations of maxima or minima of vibrational wave packets, the changing of the beating maxima or minima due to the presence of resonance from other chemical component is detrimental. A numerical comparison of vibrational beatings between a \u201cpure\u201d three excited level system of equal spacing and that of a mixture with one additional close resonant level is shown in \ufb01gure 4.1. The beating maximum of the three level system disappears when the additional level is added. Due to the coherent nature of the beating, simple subtraction of the measured beatings does not solve this problem. If the amplitude of the peak in the vibrational coherence spectrum re\ufb02ect the excitation strength and Raman cross-section of the resonance, the spectral phase around the peak in the vibrational coherence spectrum re\ufb02ects the time behavior of the resonance. With the availability of spectral phase of the vibrational coherence in the frequency domain, it is now possible to \ufb01lter out the additional \u201cimpurity\u201d resonances and Fourier transform the remaining spectrum of amplitude and phase to the time domain to reconstruct the beating response of the pure sample. The article section includes 141 \f4.2. Experiment Technique Considerations a proof-of-principle experiment on separating the vibrational beatings of mixtures. 4.2 Experiment Technique Considerations The experiment of complete characterization of molecular vibrations can be done based on a time-resolved CARS experiment setup with a pulse shaper for the probe pulse and a spectrometer with CCD. Figure 1.23 of section 1.4 shows the schematic of the setup that is used in this experiment. The complete characterization of the probe pulse is obtained through the FROG technique described in section 1.4. The accuracy of a vibrational coherence characterization depends on the accuracy of the characterization of the probe pulse. After several trials, pulse shaping of the probe pulse was found to improve the XFROG algorithm retrieval robustness and accuracy. Therefore, a \u03c0 phase step mask or sinusoidal pulse shaping was used on the probe pulse. The procedure for creating and characterizing the probe pulse is \ufb01rst to iteratively use either FROG or MIIPS and the pulse shaper to obtain a transform-limited pulse through spectral phase compensation with the pulse shaper. The FROG technique is then used to characterize the compensated probe pulse, obtaining both the amplitude and phase of the pulse. Then, the pulse shaper introduces the phase function to the compensated probe pulse, and the probe pulse is then used in the CARS process for the spectrogram generation. The discussion about the improvement of XFROG retrieval by pulse shaping of the probe pulse can be found in the published article by Konorov et.al.[6]. The XFROG algorithm is a variation of the FROG algorithm [2, 7]. Figure 4.2 illustrates the operational steps within each iteration. As the \ufb01gure shows, the XFROG algorithm necessarily requires two inputs: the two-dimensional time-frequency spectrogram I\u0005exp (\u03c9, \u03c4 ) and a well characterized probe pulse Epr (t). An initial guess is not strictly necessary but a close guess to the vibrational coherence can help the retrieval. The \ufb01rst step starts when the characterized probe pulse mathematically generates a two dimensional trace I(t, \u03c4 ) from Epr (t) with the probe pulse and the guessed 142 \f4.2. Experiment Technique Considerations Figure 4.3: This \ufb01gure shows the operational steps within the XFROG algorithm. The vibrational coherence function is represented by R(t). The probe pulse is in the time domain as Epr (t). \u03c4 is the time delay between the R(t) and probe pulse \ufb01eld. The mathematical steps are denoted as 1 to 5 and explained in text. FFT and IFFT stands for fast Fourier transform and inverse fast Fourier transform respectively. 143 \f4.2. Experiment Technique Considerations value of vibrational coherence R(t). Then the trace is Fourier transformed \u0005 \u03c4 ). This into the frequency domain to obtain calculated spectrogram I(\u03c9, calculated spectrogram is then \u201chybridized\u201d with the measured experimental spectrogram I\u0005exp (\u03c9, \u03c4 ). In this hybridization step, the amplitude of the experimental spectrogram gives the amplitude of the hybridized trace and the phase of the calculated spectrogram gives the phase of the hybridized spectrogram. After hybridization, the spectrogram is inverse Fourier transformed back to the time domain to obtain the hybrid trace I\u0005hybrid (t, \u03c4 ). This hybrid trace further undergoes the generalized projection step to provide the new generation of guess R(t). The algorithm iterates to \ufb01nd best pro\ufb01le of R(t) that produces the closest trace to the experimental recorded spectrogram. The metric minimization step is the key to the accuracy of the retrieval. It uses the same generalized projection method that is used in the FROG technique [7]. The procedure of generalized projection is to de\ufb01ne a distance metric Z and minimize it with respect to the test \ufb01eld (in the context of this chapter, R(t)). A gradient based minimization [7], is used to obtain next generation of test \ufb01eld: Z= N \u0002 ( |Iexp ti , \u03c4j ) \u2212 R(t)Epr (ti \u2212 \u03c4j )|2 (4.1) i,j=1 where Iexp (t, \u03c4 ) is the experimental trace, Etest (t) andEpr (t) are the test \ufb01eld and the well characterized probe \ufb01eld. In the actual experiment, the XFROG retrieval was done by the FROG3 software (Femtosoft). Since the software was not designed for the purpose of recovering vibrational responses, certain data format adjustment is needed. Appendix C shows the procedure for FROG3 software usage for retrieving the vibrational coherence. Appendix A includes the MATLAB simulation code that can generate the numerical CARS spectrogram and the probe pulse for the test XFROG retrieval. 144 \f4.3. Method Content 4.3 4.3.1 Method Content Overview The authors propose a new approach to vibration spectroscopy based on Coherent Anti-Stokes Raman scattering of broadband ultrashort laser pulses. The proposed method reveals both the amplitude and the phase of molecular vibrations by utilizing the cross-correlation frequency resolved optical gating (XFROG) technique. The spectrum of the anti-Stokes pulse is measured as a function of the time delay between the laser-induced molecular vibrations and a well characterized broadband femtosecond probe pulse. The iterative XFROG algorithm provides simultaneous complete characterization of molecular vibrations both in frequency and time domains with high resolution. They demonstrate experimentally the feasibility of proposed method and show one of its potential applications in disentangling the time behavior of a mixture of vibrationally excited molecules. The technique of femtosecond pulse shaping is used for further improvement of accuracy and stability against noise. 4.3.2 Content Coherent Anti-Stokes Raman Scattering (CARS) has been successfully used in spectroscopy and microscopy since the development of tuneable lasers [8, 9]. In CARS, molecular vibrations are coherently excited by the pump and Stokes pulses, and subsequently scatter the probe pulse generating the anti-Stokes signal. The temporal and spectral resolution of CARS spectroscopy is usually limited by the duration of the excitation pulses and their frequency bandwidth, respectively. Narrow bandwidth probe pulses are used in multiplex frequency-resolved CARS (fr-CARS) technique for high spectral resolution [10], whereas broadband femtosecond pulses have been employed in recent developments of time-resolved CARS (tr-CARS) spectroscopy [4, 11]. Since the time duration and the spectral bandwidth of a transform limited laser pulse are inversely proportional to each other, simultaneously 145 \f4.3. Method Content achieving high resolution in both domains requires complementary use of both fr- and tr-CARS [12, 13]. For instance, detection of the quantum beats between various vibrational frequencies of a molecule in the tr-CARS is not su\ufb03cient to recover these frequencies unambiguously, especially in the case of a large number of resonances with unknown frequency distribution. Similarly, high-resolution spectral measurement of the anti-Stokes \ufb01eld does not provide su\ufb03cient knowledge about the time response of a system. The reason for both shortcomings is the lack of information about the vibrational phase. The phase of the anti-Stokes \ufb01eld has been recently utilized for signi\ufb01cant enhancement of CARS sensitivity by means of interferometric homodyne and heterodyne detection.[14\u201318] Although the anti-Stokes phase is directly related to the phase of excited vibrational modes through the process of nonlinear frequency mixing, the latter cannot be easily retrieved from the interferometric measurements due to the presence of stochastic experimental noise. Employing spectrally narrow probe pulses (as in Refs. [14, 16]) simpli\ufb01es the problem but comes at the expense of relatively low probe power and limited frequency resolution. In this paper we show that the cross-correlation frequency resolved optical gating (XFROG) method enables robust and accurate spectral intensity and phase retrieval while using the full spectral bandwidth of the probe pulse. The improved performance of this new method stems not only from the higher available probe power but also from the redundancy of the experimental data due to the utilization of all available spectral components of the probe pulse. In the CARS process, pump pulse Ep and Stokes pulse Es coherently excite molecular vibrations with a frequency response R(\u03a9): \u0006 R(\u03a9) = \u0002 \u0007 \u0003 Ln (\u03a9) + CN R \u00b7 Ep (\u03c9 \u0004 )Es (\u03c9 \u0004 \u2212 \u03a9)d\u03c9 \u0004 (4.2) n where Ln (\u03a9) and CN R represent the contribution of the n-th resonance and the non-resonant background, respectively. The anti-Stokes \ufb01eld Eas is generated as a result of the coherent scattering of the probe pulse Epr 146 \f4.3. Method Content from the vibrations of the Raman active medium induced by the pump and Stokes \ufb01elds: Eas (\u03c9) \u221d \u0003 R(\u03a9)Epr (\u03c9 \u2212 \u03a9)d\u03a9 (4.3) The direct deconvolution of (4.3) for the retrieval of the complex vibrational response R(\u03a9) is not feasible because the experimentally measured intensity of the anti-Stokes radiation, Ias \u221d |Eas (\u03c9)|2 , loses the phase of Eas (\u03c9). A similar de-convolution problem occurs in the process of complete temporal and spectral characterization of ultrashort laser pulses,which XFROG was originally developed for [2, 19]. The XFROG iterative algorithm retrieves both the amplitude and phase of an unknown \ufb01eld E(\u03a9) = |E(\u03a9)| \u00b7 ei\u03d5(\u03a9) from its cross-correlation with a well characterized \u201cgate\u201d \ufb01eld Eg . The cross-correlation is usually performed by measuring the spectrum of a nonlinear process, such as non-resonant sum frequency generation in a nonlinear crystal, ESF G (\u03c9) \u221d \u0003 E(\u03a9)Eg (\u03c9 \u2212 \u03a9)d\u03a9 (4.4) To compensate for the missing phase of ESF G (\u03c9) in the detected intensity ISF G (\u03c9), XFROG technique introduces the time delay \u03c4 between the unknown pulse E(\u03a9) and the gate pulse Eg , and applies an iterative retrieval algorithm to the acquired two-dimensional spectrogram ISF G (\u03c9, \u03c4 ). The desired solution E(\u03a9) is found by means of the mathematical procedure known as the method of generalized projections [19]. By iteratively projecting onto the well de\ufb01ned constraint sets both in the time and frequency domains, in all practical cases the method leads to a unique solution for E(\u03a9). The robustness of the XFROG algorithm stems from the redundancy of the two-dimensional scan which contains (quadratically) more data points than there are unknowns in the sought solution E(\u03a9). This high degree of redundancy enables complete reconstruction of E(\u03a9) from the measured ISF G (\u03c9, \u03c4 ). The similarity of expressions (4.3) and (4.4) suggests the possibility of de-convolving R(\u03a9) by means of the XFROG technique. Indeed, the coherent molecular vibration response R(\u03a9) in (4.3) is analogous to the unknown pulse E(\u03a9) in (4.4). In the CARS process, these coherent vibrations are \u201cmixed\u201d with the probe pulse to produce the third order polarization 147 \f1e5 10 1e4 9 1e3 8 1e2 7 1e1 6 1 5 4 3 2 1 0 -1 -2 720 730 740 750 Anti-Stokes wavelength (nm) 5 10 (b) 8 4 3 6 2 4 1 2 0 Phase (rad) (a) Amp. square (a.u.) Probe time delay (ps) 11 0 900 1000 1100 1200 1300 Raman shift (cm-1) (c) 8 4 6 3 4 2 2 1 0 Phase (rad) 12 Amp. square(a.u.) 4.3. Method Content 0 0 1 2 3 4 5 6 Time (ps) Figure 4.4: (Color online). (a) Numerical simulation of the frequency resolved CARS spectrogram for Toluene molecule (log scale). \u03c0-step spectral phase shaping has been applied to a gaussian probe pulse with the spectral bandwidth of 10nm (FWHM), resulting in sharp interference fringes which serve as \u201cfrequency markers\u201d for the XFROG retrieval algorithm (see text). (b,c) XFROG retrieval of the square of the amplitude (thin black) and the phase (thick blue) of the vibrational response in frequency and time domains, respectively. which generates the observable anti-Stokes pulse Eas (\u03c9), in direct analogy with the sum frequency generation in a nonlinear crystal. Following this analogy, we introduced the time delay between the pump-Stokes pulse pair and the probe pulse, and applied the iterative XFROG algorithm to the two-dimensional CARS spectrogram Ias (\u03c9, \u03c4 ) \u221d |Eas (\u03c9, \u03c4 )|2 , where Eas (\u03c9, \u03c4 ) \u221d \u0003 R(\u03a9)Epr (\u03c9 \u2212 \u03a9)e\u2212i\u03a9\u03c4 d\u03a9 (4.5) Numerical simulations of the CARS spectrogram Ias (\u03c9, \u03c4 ) for Toluene molecule are shown in \ufb01g.4.4(a). We used commercial XFROG software package (FROG3, Femtosoft Technologies) to extract the complex vibrational response R(\u03a9) in frequency and time domains, shown in \ufb01g.4.4(b) 148 \f4.3. Method Content and \ufb01g.4.4(c), respectively. The retrieved positions of the resonances agree with the values used for calculating the spectrogram. The amplitude of each resonant line is determined by the input resonance strength and by the spectral power of the pump-Stokes \ufb01eld correlation at the corresponding resonance frequency. Three resonances at 1000 cm\u22121 , 1027 cm\u22121 and 1206 cm\u22121 are clearly resolved. Phase dips at the location of each resonance agree with the assumed Lorentzian model of the resonant molecular response. The latter implies that Cn (\u03a9) = Cn \/ (\u03a9 \u2212 \u03a9n + i\u0393n ), where Cn , \u03a9n and \u0393n are the strength, the frequency and the width of the n-th resonance. Our numerical analysis shows that the XFROG algorithm becomes less susceptible to noise with the increased number of sharp features in the input spectrogram [6]. Such features, or \u201cfrequency markers\u201d, can be introduced by means of the spectral phase shaping of the probe pulse. The latter involves controlled modi\ufb01cation of the spectral phase of the pulse \u0004 (\u03c9) = by applying an external phase function \u03c6(\u03c9) to its spectrum, i.e. Epr Epr (\u03c9)\u00d7ei\u03c6(\u03c9) . A simple, yet very useful, spectral shape consists of a \u03c0 -step at the central frequency of the pulse \u03c90 . That is, \u03c6(\u03c9) = 0 if \u03c9 < \u03c90 , and \u03c6(\u03c9) = \u03c0 otherwise. The e\ufb00ect of the \u03c0-step phase shaping on resonantly enhanced multiphoton processes, such as CARS or two-photon absorption, has been thoroughly discussed and exploited in a series of works by Silberberg and co-workers [14, 20]. In the time domain, the \u03c0-step shaping splits an originally transform limited pulse into a pair of phase-coherent pulses. The two corresponding anti-Stokes \ufb01elds generated by this probe pair interfere as long as the coherent excitation is preserved in the medium due to the presence of vibrational resonances. The interference fringes, seen on the spectrogram as sharp edges along the time axis (\ufb01g. 4.4(a)), serve as the frequency markers of the Raman lines and help the XFROG algorithm determine the absolute position of the resonances. We will discuss the performance of di\ufb00erent pulse shapes in a follow-up paper [6]. The experimental results of the frequency resolved CARS gating method with the spectrally shaped probe pulse are shown in \ufb01g.4.5. We used a commercial Ti-Sapphire regenerative ampli\ufb01er system (SpitFire, SpectraPhysics) generating pulses of \u223c10nm bandwidth (FWHM), a tuneable opti149 \f4.3. Method Content cal parametric ampli\ufb01er (TOPAS, Light Conversion), and a home built pulse shaper based on a liquid crystal spatial light modulator (SLM-128, CRI) and implemented in a commonly used 4f design [21]. The central wavelengths were set to 1111 nm, 1250 nm and 800 nm, for the pump, Stokes and probe pulse, respectively. The pulse shaper was \ufb01rst utilized for \ufb02attening the spectral phase of the probe pulse. This transform limited probe was used either directly or after an additional phase shaping was applied by the pulse shaper. Incident pulses with energies lower than 10\u03bcJ were focused in the BOXCARS phase matching geometry on a liquid sample held in 5 mm optical path quartz cuvette. Low average power pulses are su\ufb03cient to generate enough CARS signal because this method utilize full bandwidth of laser as probe pulses. The generated CARS signal was spatially \ufb01ltered from the residual excitation beams and coupled into a spectrometer with a spectral resolution of 0.05 nm. The time delay \u03c4 between the probe pulse and the pump-Stokes pair was scanned in 20 fs steps. The results of the XFROG retrieval of the spectral amplitude and phase of the vibrational response R(\u03a9) are shown in \ufb01g.4.5(b). Con\ufb01rming our numerical analysis, the experiment shows that the resolution is improved when the shaped probe pulse was used, as opposed to the case of the unshaped transform limited probe [6]. The positions of the three resonance peaks (at 1000 cm\u22121 , 1027 cm\u22121 and 1206 cm\u22121 ) are in good agreement with the reference spectrum of spontaneous Raman scattering shown by the red dashed line. The peak intensities depend on the spectral power density of the pump-Stokes \ufb01eld correlation at the corresponding frequency \u03a9, as well as the scattering cross section, and are therefore higher at the central frequency of 1000 cm\u22121 . The central peak has a FWHM of \u223c3 cm\u22121 , signi\ufb01cantly sharper than the bandwidth of our probe pulse of \u223c170 cm\u22121 , and is even comparable to spontaneous Raman spectrum. In the simultaneously retrieved time response shown in \ufb01g.4.5(c), coherent oscillations with a period of 160 fs are clearly observed, con\ufb01rming that the time resolution of the XFROG retrieval is determined by the broad spectral bandwidth of the molecular nonlinear response and the probe pulse bandwidth, rather than by the probe pulse duration which in the case of the \u03c0-step shaping 150 \f1e5 Probe time delay (ps) 11 1e4 10 1e3 9 1e2 8 7 1e1 6 1 5 4 3 2 1 0 -1 -2 720 730 740 750 Anti-Stokes wavelength (nm) 10 4 2 (b) 8 3 0 990 6 1020 2 4 1 2 Phase (rad) (a) 0 0 900 3 (c) 1000 1100 1200 1300 Raman shift (cm-1) 4 3 2 2 1 1 0 0 1 2 3 4 5 6 Phase (rad) 12 Amp. square (a.u.) Amp. square (a.u.) 4.3. Method Content 0 Time (ps) Figure 4.5: (Color online). (a) Experimental frequency resolved CARS spectrogram for Toluene sample with the spectrally shaped probe pulse (\u03c0 \u2212 step at 800 nm, log scale). (b,c) XFROG retrieval of the square of the amplitude (thin black) and phase (thick blue) of the vibrational response in frequency and time domains, respectively. Dashed red line in (b) represents the reference spectrum of spontaneous Raman scattering from the same sample. Zoom-in to the central part of the spectrum is shown in the inset in plot (b). exceeds 500 fs. Spectral phase shifts are observed across each resonant line as expected from the Lorentzian model. The magnitude of the phase shifts is lower than \u03c0 radian due to the presence of the non-resonant background. Being a result of a coherent process, anti-Stokes \ufb01elds generated by multiple vibrational resonances interfere and therefore cannot be separated unless both the amplitude and the phase of the total vibrational response are known. The key ability of the proposed method to reveal the phase of molecular vibrations is demonstrated by applying the method to the indirect retrieval of the vibrational response of a molecule from the measured response of its mixture with another molecular species. Such a task would be particularly important if the mixture cannot be separated, and the collective Raman response represents the only available spectroscopic data. 151 \f4.3. Method Content We demonstrate this by retrieving the vibrations of Toluene from the measured CARS spectrogram of its mixture with orto-Xylene as shown in \ufb01g.4.6. XFROG retrieval of the time and frequency response of the mixture is shown in plots (a) and (b), respectively. In the absence of the phase information, masking the three main resonances of orto-Xylene at 982 cm\u22121 , 1049 cm\u22121 and 1220 cm\u22121 is not su\ufb03cient for reconstructing the complex Raman response of Toluene because the inverse Fourier transform from the frequency into the time domain cannot be carried out properly. The availability of the phase in our XFROG retrieval, however, makes this procedure possible. We masked out the three resonances of orto-Xylene in the complex spectrum of the mixture by substituting the amplitude and the phase in their vicinity by a linear slope connecting the two values at the two sides of each resonance (shaded regions in (b)). The Fourier transform of the resulting complex spectrum is compared with the direct XFROG retrieval of the temporal vibrational response of pure Toluene in \ufb01g.4.6(a). As shown by the close-up in \ufb01g.4.6(c), excellent agreement between the direct retrieval from the pure sample (thin blue) and indirect retrieval from the mixture (thick black) on the time scale of a few picoseconds demonstrates the potential of the proposed technique as a new tool for studying molecular dynamics in complex environments. The limitations and possible sources of error of the proposed method of XFROG CARS can be seen from the analysis of equations. (4.2) and (4.5). The former assumes that a single vibrational ground state is coupled to a set of excited vibrational levels via nonresonant two-photon transitions by a two-photon \ufb01eld Ep (t)Es (t). We \ufb01rst note that the complex response R(\u03a9) re\ufb02ects not only the inherent properties of the medium described by the term in the square brackets in Eq. 4.2 but also the \ufb01eld characteristics of the pump and Stokes pulses. For instance, a small residual frequency chirp in the pump-Stokes \ufb01eld correlation can be seen in Fig. 4.5(b) as a small parabolic background. Furthermore, any intermediate one-photon resonance at the pump or Stokes frequency will change the phase and amplitude of R(\u03a9). However, owing to the preserved coherence of the excitation, the XFROG retrieval, though more complicated, will properly re\ufb02ect the 152 \fAmplitude of Raman response (a.u.) 4.3. Method Content 10 (a) 7 8 (b) 6 6 4 5 2 0 900 4 950 1000 1050 1100 1150 1200 1250 Raman shift (cm-1) 2.5 3 2 2 (c) 1.5 1 1 0.5 0 0 0.5 1 1.5 2 2.5 3 Time (ps) 3.5 4 4.5 5 0 2 2.5 3 3.5 4 4.5 5 Time (ps) Figure 4.6: (Color online). (a) XFROG retrieval of the vibrational oscillations of Toluene (two upper curves, shifted for clarity), and of the mixture of Toluene with orto-Xylene (lower red curve). The two upper curves were obtained by the direct retrieval from pure Toluene (middle blue) and by the indirect reconstruction of the same response from the collective response of the mixture (top black). (b) XFROG retrieval of the complex spectrum of the mixture. Both amplitude (thin black) and phase (thick blue) around the three strong resonances of orto-Xylene (shaded rectangles) were masked for the complete reconstruction of the Raman response of Toluene by the Fourier transform of the modi\ufb01ed complex spectrum. (c) Close comparison of the directly (thin blue) and indirectly (thick black) retrieved vibrational amplitude of Toluene from the pure sample and mixture, respectively. Vibrational response of the mixture is shown by the dashed red curve for reference. 153 \f4.3. Method Content induced molecular vibration. On the other hand, an incoherent mixture of initially populated ground levels will result in faster dephasing of the ensemble-averaged coherences and cause an e\ufb00ective broadening of the vibrational lines. Similar analysis of Eq. 4.5 shows that the XFROG algorithm is applicable only to the case of non-resonant scattering of the probe pulse. Moreover, any discrepancy between the real probe and the one used as an input to the XFROG calculations reduces the accuracy of the amplitudephase retrieval. We also note that the proposed technique is not limited to the vibrations in the electronic ground state, as it can be used for the analysis of any long-lived vibrations accessible through a two-photon excitation in a general four-wave mixing process. In principle, it can be applied not only to CARS but also to other coherent interaction schemes. In conclusion, we demonstrated the frequency resolved gating of molecular vibrations as a highly e\ufb00ective and robust method of simultaneous revealing the amplitude and the phase of molecular vibrations. The ability to use full spectral bandwidth of the femtosecond probe pulses, o\ufb00ered by the XFROG CARS, results in higher signal-to-noise ratios, lower required probe power, and high stability against noise. The latter is enhanced by the redundancy of the XFROG retrieval, which is based on simultaneous processing of multiple anti-Stokes signals generated by all spectral components of the probe pulse. Unlike the interferometric methods of phase sensitive detection, the XFROG technique retrieves the phase of molecular vibrations, rather than the phase of the anti-Stokes \ufb01eld. The availability of the vibrational phase provides additional information about the system and extends our capabilities of studying its dynamics. The method is demonstrated experimentally by successfully separating temporal Raman responses of two mixed molecular species without physically separating the mixture. The utilization of femtosecond pulse shaping technique further improves the performance of this method. 154 \fBibliography [1] J. K. Kauppinen, D. J. Mo\ufb00att, H. H. Mantsch, and D. G. Cameron, Applied Spectroscopy 35, 271 (1981). [2] S. Linden, H. Giessen, and J. Kuhl, Physica Status Solidi B-Basic Research 206, 119 (1998). [3] M. Schmitt, G. Knopp, A. Materny, and W. Kiefer, Journal of Physical Chemistry A 102, 4059 (1998). [4] T. Lang, K. L. Kompa, and M. Motzkus, Chemical Physics Letters 310, 65 (1999). [5] G. Knopp, I. Pinkas, and Y. Prior, Journal of Raman Spectroscopy 31, 51 (2000). [6] S. O. Konorov, X. G. Xu, R. F. B. Turner, M. W. Blades, J. W. Hepburn, and V. Milner, Optics Express 15, 7564 (2007). [7] K. W. Delong, D. N. Fittingho\ufb00, R. Trebino, B. Kohler, and K. Wilson, Optics Letters 19, 2152 (1994). [8] W. M. Tolles, J. W. Nibler, J. R. McDonald, and A. B. Harvey, Applied Spectroscopy 31, 253 (1977). [9] J. X. Cheng and X. S. Xie, Journal of Physical Chemistry B 108, 827 (2004). [10] J. X. Cheng, A. Volkmer, L. D. Book, and X. S. Xie, Journal of Physical Chemistry B 106, 8493 (2002). [11] M. Schmitt, G. Knopp, A. Materny, and W. Kiefer, Chemical Physics Letters 270, 9 (1997). [12] M. Heid, S. Schlucker, U. Schmitt, T. Chen, R. Schweitzer-Stenner, V. Engel, and W. Kiefer, Journal of Raman Spectroscopy 32, 771 (2001). 155 \fChapter 4. Bibliography [13] B. D. Prince, A. Chakraborty, B. M. Prince, and H. U. Stau\ufb00er, Journal of Chemical Physics 125 (2006). [14] D. Oron, N. Dudovich, and Y. Silberberg, Physical Review Letters 89 (2002). [15] D. L. Marks, C. Vinegoni, J. S. Bredfeldt, and S. A. Boppart, Applied Physics Letters 85, 5787 (2004). [16] S. H. Lim, A. G. Caster, and S. R. Leone, Physical Review A 72 (2005). [17] M. Cui, J. P. Skodack, and J. P. Ogilvie, Biophysical Journal pp. 197A\u2013 197A (2007). [18] E. O. Potma, C. L. Evans, and X. S. Xie, Optics Letters 31, 241 (2006). [19] K. W. Delong, R. Trebino, J. Hunter, and W. E. White, Journal of the Optical Society of America B-Optical Physics 11, 2206 (1994). [20] N. Dudovich, B. Dayan, S. M. G. Faeder, and Y. Silberberg, Physical Review Letters 86, 47 (2001). [21] A. M. Weiner, Review of Scienti\ufb01c Instruments 71, 1929 (2000). 156 \fChapter 5 Background-free Coherent Raman Spectroscopy by Detecting the Spectral Phase of Molecular Vibrations 5.1 Motivation CARS spectroscopy has many advantages over spontaneous Raman spectroscopy such as high signal strength, low \ufb02uorescence background and directional signals. However, the disadvantage of high non-resonant background in CARS limits its application. Due to the universal existence of \u03c7(3) , CARS has non-resonant Four-Wave-Mixing background independent of the presence of resonances. The problems are twofold for CARS with broad band pulses. Firstly, the presence of non-resonant background at the same frequency as the resonances creates the dispersive line pro\ufb01les in the vibrational coherence R(\u03a9). For CARS methods with narrow band probing, where the CARS spectrum re\ufb02ects the pro\ufb01le of R(\u03a9), dispersive pro\ufb01les complicate peak \ufb01tting. In addition, for CARS methods with broad band probing, the frequency components in the CARS spectrum can come from both resonant contributions and non-resonant response of di\ufb00erent frequencies. This is shown in \ufb01gure 5.1, where the broadband probe pulse links 0 A version of this chapter has been published as Xiaoji G. Xu, Stanislav O. Konorov, John. W. Hepburn and Valery Milner \u201cBackground-free Coherent Raman Spectroscopy by Detecting the Spectral Phase of Molecular Vibrations\u201dOptics Letters vol. 33 page 1177-1179. 2008 157 \f5.1. Motivation E e (B) (A) CARS c CARS Probe Stokes pump d probe a b Vibrational coherence \u0004 Figure 5.1: The energy level diagram is shown in \ufb01gure (A). The convolution e\ufb00ect of CARS signal with high non-resonant background and broad band probing is shown in \ufb01gure (B). The frequency contribution from resonance (a) (speci\ufb01ed by an arrow) interacts with frequency component (c) from a broad band probe pulse and contributes to the CARS frequency at location e. However the non-resonant response at position (b) interacts with frequency component (d) and also contributes to the same CARS signal at (e). 158 \f5.1. Motivation both resonant level and non-resonant response to the same frequency component in the CARS spectrum. This problem can also be regarded as a continuation of the convolution problem that is discussed in chapter 4. The non-resonant response adds a background to the vibrational coherence R(\u03a9) and this background participates in the convolution process with a broad band probe pulse. For CARS techniques with narrow-band probe pulses, i.e. multiplex CARS, polarization has been used to remove the non-resonant signal contribution [1, 2], based on a small angle polarization di\ufb00erence between resonant CARS and non-resonant background. This method works in such a way that the polarizer is orthogonal to the polarization of non-resonant FWHM signal, so the optical signal passing through the polarizer is purely from the resonant CARS signal. However, the polarization di\ufb00erence of the resonant CARS signal and the non-resonant FWM signal is often about 5-10\u25e6 . When blocking the non-resonant signal, the majority of resonant signal is also blocked, therefore the utilization of polarization \ufb01ltering leads to severe attenuation of the resonant signal. Broad band time-resolved CARS, on the other hand, can avoid non-resonant background quite easily if the short duration probe pulse is properly time-delayed with respect to the excitation pair. However, as mentioned in the discussion in section 1.2, time-resolved CARS gives only the vibrational level spacing of the sample. To solve the non-resonant background problem in CARS with broad band pulses, a spectral phase approach based on complete characterization of molecular vibrations was proposed and demonstrated [3]. The complete characterization of molecular vibrations technique can e\ufb00ectively remove the convolution e\ufb00ect introduced by the broad band probe pulse, therefore solving the convolution problem between the resonant spectra and non-resonant background. In addition to the application of complete characterization of molecular vibrations method, this chapter solves the non-resonant background problem of CARS by detecting the spectral phase. When the nonresonant background is high, the retrieved spectral phase pro\ufb01le of the vibrational coherence is a good approximation of the spectrum of vibrational resonances. 159 \f5.1. Motivation The spectral phase \u03a6 of the vibrational coherence R(\u03a9) is related to the ratio between the imaginary part of R(\u03a9) and the real part of R(\u03a9) by arctan[ Im(R(\u03a9)) Re(R(\u03a9)) ]. As discussed in section 3.2.1 and shown \ufb01gure 1.16, the imaginary part of R(\u03a9) re\ufb02ects the pro\ufb01le of the vibrational resonances of the sample. The real part of R(\u03a9), however, comes from both the real part of the resonance and non-resonant background. The overall spectrum of R(\u03a9) often has dispersive pro\ufb01les. As equation 1.41 shows, the non-resonant background adds a real number CnR to R(\u03a9). When the non-resonant background is high, the real part of R(\u03a9) is going to re\ufb02ect primarily the high value of the non-resonant contribution, whereas the imaginary part of R(\u03a9) remains the same. As a result, the spectral phase \u03a6 can be approximated by Im(R(\u03a9)) Re(R(\u03a9)) . Now the Re(R(\u03a9)) is primarily CnR times a \ufb01eld correlation fac- tor A(\u03a9). Consequently, the spectral phase \u03a6 of the vibrational coherence R(\u03a9) re\ufb02ects the imaginary part of the vibrational coherence divided by the \ufb01eld correlation A(\u03a9) and gives the pro\ufb01le of the vibrational resonances. A point worth noting about this spectral phase approach is the ratio between the non-resonant background and the resonant contribution. For the spectral phase to have similar pro\ufb01le as the imaginary part of the the vibrational coherence, the non-resonant background should be high, at least comparable to the strength of the resonant response. The comparison of the spectral phase and the total spectrum of R(\u03a9) is shown in \ufb01gure 5.2. When \u00af the non-resonant background is high (100% in \ufb01gure 5.2(A) and 50% in (B)) \u00af the spectral phase re\ufb02ects the peak pro\ufb01le of the resonances. When the the non-resonant background is low (10% in \ufb01gure 5.2(C) the spectral phase \u00af shows severe distortion comparing to pro\ufb01le of the vibrational resonance as shown in \ufb01gure 5.2(D). This means when non-resonant background is low, \u00af the spectral phase of R(\u03a9) cannot be safely used as the pro\ufb01le of the vibrational resonance. A practical estimation on the threshold non-resonant background to resonant response ratio is 50%; if the non-resonant background is about 50% of the strength of resonant response, the spectral phase approach can be used and peaks on the spectral phase has correct linewidths and relevant intensity to that of the vibrational resonances. If the non-resonant background is low, the linewdith and intensity shows severe distortion that 160 \f5.1. Motivation 15 15 Intensity (AU) A B 10 10 5 5 0 500 15 1000 1500 500 1000 1500 1000 1500 D C 10 5 0 500 1000 1500 500 Wave number (cm-1) Figure 5.2: Figure A, B and C show the comparisons between spectral phase (red thick line) and total intensity (blue thin line) of R(\u03a9). (A) the nonresonant background has the same peak value as the resonant response. (B) the non-resonant background has 50% peak value as the resonant response. (C) the non-resonant background has 10% peak value as the resonant response. Figure (D) is the plot of the imaginary part of resonant response that corresponds to vibrational resonances. 161 \f5.2. Method Content cannot be taken as the indication of linewdith and intensities of vibrational resonances. However, when the non-resonant background is low, the total spectrum of the vibrational coherence can be directly used as the spectrum of the vibrational resonances and there is no need to use the proposed spectral phase approach method. In CARS experiments of condensed phase samples, the non-resonant background depends on the properties sample. Toluene, a commonly used strong Raman active sample, has an estimated ratio of 20% between the strength of non-resonant response and that of the resonant response. For other sample, this ratio can be assumed to be higher than that of toluene. The spectral phase approach is an e\ufb00ective way of removing high nonresonant background of CARS. It is an application of complete characterization of molecular vibration method. It is speci\ufb01cally useful for those samples that have high non-resonant background. Unlike the polarization techniques, the spectral phase approach detects all the CARS signals. Therefore it can be applied to samples with low total signal. The article section is going to show expression derivations and experiment demonstrations in detail. 5.2 5.2.1 Method Content Overview The authors propose and demonstrate a new approach to subtracting high non-resonant background in coherent anti-Stokes Raman Scattering (CARS) spectroscopy. The method is based on the retrieval of the spectral phase of molecular vibrations using the technique of frequency resolved optical gating of Raman scattering. In the presence of high non-resonant background, the retrieved phase corresponds directly to the background-free spectrum of the coherent Raman response. 5.2.2 Content Since its discovery [4, 5], coherent anti-Stokes Raman scattering (CARS) has been widely used for vibrational spectroscopy. In recent years, CARS 162 \f5.2. Method Content spectroscopy has attracted signi\ufb01cant attention because of its applications in biological imaging [6, 7] and chemical diagnosis [8]. However, the often present instantaneous non-resonant background interferes with and typically dominates the much weaker resonant response, making an accurate retrieval of the CARS spectrum di\ufb03cult. Commonly employed polarization \ufb01ltering, though successful in removing the non-resonant signal [1, 2], signi\ufb01cantly attenuates resonant contribution thus reducing the signal-to-noise ratio. An alternative approach based on heterodyne detection [9\u201312] comes at the expense of high experimental complexity and requires interferometrical stability of optical components. The non-resonant background can also be eliminated by properly delaying the probe pulse in time resolved CARS [13, 14]. This method, however, is susceptible to imperfect spectral phase of the excitation pulses. Here, we present a simple and robust experimental approach which enables an accurate retrieval of the coherent Raman spectrum in the presence of high non-resonant response. Coherent anti-Stokes Raman scattering is a four-wave-mixing process, in which the coherent vibrational response R(\u03a9) is excited by the two-photon \ufb01eld A(\u03a9) of the pump and Stokes photons: \u0006 R(\u03a9) = \u0002 k \u0007 Ck + Cnr \u00d7 A(\u03a9), \u03a9 \u2212 \u03a9k \u2212 i\u0393k where \u0003 A(\u03a9) = Ep (\u03c9 \u0004 )ES\u2217 (\u03c9 \u0004 \u2212 \u03a9)d\u03c9 \u0004 . (5.1) (5.2) Vibrational coherence is prepared when the pump and Stokes excitation \ufb01elds, Ep (\u03c9) and ES (\u03c9), respectively, overlap temporally and spatially on a Raman active sample. Equation (5.1) assumes a Lorentzian resonant response with \u03a9n , \u0393n and Cn being the position, linewidth and strength of the k\u2212th resonance, whereas Cnr represents the non-resonant contribution. CARS signal, ECARS , results from the scattering of the probe pulse, Epr (\u03c9), o\ufb00 the excited vibrational coherence R(\u03a9). In the case of spectrally broad pulses, this can be expressed as a \ufb01eld correlation in the frequency 163 \f5.2. Method Content domain: ECARS (\u03c9) \u221d \u0003 R(\u03a9)Epr (\u03c9 \u2212 \u03a9)d\u03a9 (5.3) The non-resonant background Cnr is a real number which can be assumed frequency-independent across the excitation bandwidth. The coherent nature of the vibrational response results in the interference of the resonant and non-resonant terms in the scattering process described by Eq. (5.3). Figure 5.3 shows the numerical simulation of both the squared amplitude (|R(\u03a9)|2 ) and phase (\u03a6(\u03a9)) of the complex vibrational response based on the spectroscopic data for azobenzene. As seen in Fig. 5.3(a), high nonresonant background distorts the lineshape of the small resonance around 1319 cm\u22121 into a characteristic dispersion pro\ufb01le. Such distortion represents a common problem both in narrowband and broadband CARS experiments as it creates ambiguity in the peak \ufb01tting and complicates the comparison between the coherent and spontaneous Raman spectra, often required for line identi\ufb01cation. Here, we present an alternative approach to subtracting high non-resonant background in CARS spectroscopy. The spectral phase of R(\u03a9) can be expressed as \u03a6(\u03a9) = arctan Im(R(\u03a9)) Im(R(\u03a9)) \u2248 , Re(R(\u03a9)) Re(R(\u03a9)) (5.4) where the approximate equality holds in the limit of Im(R(\u03a9)) << Re(R(\u03a9)). As seen from Eq. 5.1, this limit is reached in the case of high non-resonant response, i.e. when Cnr >> Ck \/\u0393k , and transform-limited excitation, i.e. when the pump-Stokes \ufb01eld correlation A(\u03a9) is a real quantity. Neglecting the real part of the resonant response, outweighed by Cnr , we arrive at: \u0006 \u03a6(\u03a9) \u2248 \u0002 k \u0007 Ck \u0393k \/Cnr . (\u03a9 \u2212 \u03a9k )2 + \u03932 (5.5) Hence, the resonant Raman spectrum, represented by the sum in the square brackets, is directly proportional to the spectral phase \u03a6(\u03a9). This correspondence can be seen in comparing the spectral phase with the Raman spectrum in the numerically simulated cases of strong and zero non-resonance back164 \f1.0 (a) 6 (b) 4 0.8 Phase (rad) Amplitude square (a.u.) 5.2. Method Content 2 0.6 0 0.4 0.2 -2 0 -4 1000 1200 1400 1600 1000 Raman shift 1200 1400 1600 (cm-1) Figure 5.3: (Color online) Numerical simulation of the squared amplitude (solid black) and phase (dashed blue) of coherent vibrational response of azobenzene with (a) and without (b) high non-resonant background excited by the pump and Stokes pulses of 130 fs duration (fwhm). The similarity between the phase in (a) and amplitude in (b) is the key point exploited in our approach to background subtraction. ground (Figs. 5.3(a) and 5.3(b), respectively). Note, that as long as the excitation \ufb01eld A(\u03a9) is real, its spectral pro\ufb01le does not enter the proportionality between the spectral phase and the Raman spectrum (Eq. (5.5)). Therefore, the relative strength of various Raman modes, Ck , is properly re\ufb02ected in \u03a6(\u03a9), regardless of their spectral overlap with the excitation pro\ufb01le A(\u03a9). This property makes the spectral phase more convenient quantity than the imaginary part of R(\u03a9) which, being proportional to A(\u03a9), favors the central part of the excitation spectrum. Detecting the spectral phase of the vibrational response R(\u03a9) is not a trivial task. One way of extracting the vibrational phase from the time- and frequency-resolved CARS measurements has been recently demonstrated by our group [3]. The method utilizes the retrieval algorithm of crosscorrelation frequency resolved optical gating (XFROG) applied to the ex- 165 \f5.2. Method Content perimentally measured two-dimensional time-frequency CARS spectrogram. Here, we implement the XFROG-CARS technique for e\ufb03cient background subtraction from the experimentally detected vibrational spectrum of azobenzene. Because of the gas sample that we used in this work, the experiment was carried out with a regenerative Ti-Sapphire ampli\ufb01er (Spit\ufb01re, SpectraPhysics, pulse duration of 130 fs (fwhm), 1 kHz repetition rate) which provided 800nm wavelength probe pulses, and an optical parametric ampli\ufb01er (TOPAS, Light Conversion) generating the pump and Stokes pulses at the wavelength of 1080nm and 1270nm, respectively. All laser beams were focused with a 50 cm focal-length lens to overlap in the boxcars phasematching geometry [15] inside a gas cell \ufb01lled with azobenzene and heated to \u2248 500 K (vapor pressure 18kpa). The anti-Stokes beam was spatially \ufb01ltered and coupled into a spectrometer (McPherson 2035) with a CCD detector (Andor iDus 401DV). Two-dimensional CARS spectrograms were recorded by detecting the anti-Stokes spectrum while scanning the time delay between the probe and synchronized pump-Stokes pulse pair by a motorized translation stage. The total recording time of one spectrogram ranges from two to ten minutes, depending on the required resolution and limited by the sensitivity of the detector. A typical experimental spectrogram is shown in \ufb01gure 5.4. Excited Raman modes result in the long tail on the picosecond time scale, while the instantaneous non-resonant response contributes to the sharp spike(s) at three pulses overlap. The spectrograms were used as an input to the commercial XFROG software (FROG3, FemtoSoft) for the retrieval of the amplitude and phase of the vibrational response R(\u03a9) as described in reference [3]. To improve the performance of the XFROG technique, the probe pulses were spectrally shaped with a home made pulse shaper based on a liquid crystal spatial light modulator. The pulse shaper was used for \ufb02attening the spectral phase of the probe pulse. Sinusoidal phase modulation was then applied to the transform limited probe by means of the same pulse shaper, resulting in a rich interference pattern in the measured two-dimensional CARS spectrogram (Fig. 5.4). Detailed discussion on this shaping can be 166 \f5.2. Method Content Probe time delay (ps) 6 1e5 1e4 1e3 1e2 1e1 1 5 4 3 2 1 0 -1 -2 710 720 730 740 750 Wavelength (nm) Figure 5.4: Experimentally observed time-frequency CARS spectrogram of azobenzene. (Details see text) found in our earlier paper [16]. The results of the XFROG processing of the recorded CARS spectrogram are shown in Fig. 5.5(a). As re\ufb02ected by the big pedestal around the center of the pump-Stokes excitation spectrum (\u223c 1300 cm\u22121 ), the vibrational response of azobenzene exhibits strong non-resonant background in this spectral region. Hence, the small resonance around 1319 cm\u22121 assumes a characteristic dispersive pro\ufb01le. On the other hand, the retrieved spectral phase of R(\u03a9) shows much better correspondence to the locations and lineshapes of the Raman peaks, as illustrated in Fig. 5.5(b). Here, the smoothly changing baseline has been removed from the retrieved \u03a6(\u03a9). The curvature of this baseline re\ufb02ects the residual frequency chirp of the pump-Stokes convolution \ufb01eld (see Eq. (5.2)). As a result, di\ufb00erent parts of the vibrational spectrum are excited at slightly di\ufb00erent time moments. In direct analogy to chirp photon \ufb01eld, this results in an e\ufb00ective chirp of the coherent vibrational response which appears as a parabolic o\ufb00set to \u03a6(\u03a9). 167 \f5.2. Method Content 2 1.2 (b) 0 -2 0.8 -4 0.4 Phase (rad) Amplitude square (a.u.) (a) -6 0 1000 1200 1400 1600 -8 1200 1400 1600 Raman shift (cm-1) Figure 5.5: (Color online) (a) XFROG retrieval of the squared amplitude, |R(\u03a9)|2 (solid black), and phase, \u03a6(\u03a9) (dashed blue), of the coherent Raman response of azobenzene. Sharp dips in the spectral phase correspond to the Raman resonances. Smooth parabolic baseline indicates the residual frequency chirp of the pump-Stokes pulses. (b) The retrieved spectral phase (upper red) in comparison with the spontaneous Raman spectrum (middle blue) and the squared amplitude of the vibrational response R(\u03a9) (lower black). The background-free spectral phase better re\ufb02ects the small peaks at 1317 cm\u22121 and 1591 cm\u22121 (dashed lines), whereas |R(\u03a9)|2 shows dispersive pro\ufb01les on top of the strong non-resonant background. Such phase curvature can be easily subtracted by performing a separate characterization of the excitation pulses and compensated. After the removal of the slow varying baseline, the retrieved spectral phase shows close resemblance to the spontaneous Raman spectrum, as illustrated in \ufb01g. 5.5(b). Our spectral phase approach demonstrates good sensitivity by revealing the 1591 cm\u22121 peak on the far side of the excitation band. As expected, the spectral resolution is de\ufb01ned by the length of the time-delay scan rather than the probe bandwidth (the latter being about 130 cm\u22121 ). Note, that although the approximation of high non-resonant background invoked in this work is not necessarily valid across the whole spectrum, the agreement between the retrieved spectral phase, \u03a6(\u03a9), and 168 \f5.2. Method Content the reference spectrum of spontaneous Raman is very satisfactory. The deviations can be seen in the incorrect relative strength of the side peaks (e.g. 1493 cm\u22121 ) whose amplitude is comparable to that of the non-resonant background. In conclusion, we have demonstrated a new approach to remove high nonresonant background in CARS spectroscopy, based on the detection of the spectral phase of the vibrational response by means of the recently developed XFROG-CARS technique. The method proves applicable as long as the non-resonant response is comparable to or stronger than the amplitude of Raman resonances. The suggested technique does not require narrowband probing, and does not rely on polarization \ufb01ltering or optical interferometry. In principle, it can be implemented in the collinear geometry and utilized in CARS microscopy, if the acquisition time is shortened to within practical limits. 169 \fBibliography [1] J. X. Cheng, L. D. Book, and X. S. Xie, Optics Letters 26, 1341 (2001). [2] N. I. Koroteev, M. Endemann, and R. L. Byer, Physical Review Letters 43, 398 (1979). [3] X. J. G. Xu, S. O. Konorov, S. Zhdanovich, J. W. Hepburn, and V. Milner, Journal of Chemical Physics 126 (2007). [4] P. D. Maker and R. W. Terhune, Physical Review 137, A801 (1965). [5] W. M. Tolles, J. W. Nibler, J. R. McDonald, and A. B. Harvey, Applied Spectroscopy 31, 253 (1977). [6] J. X. Cheng and X. S. Xie, Journal of Physical Chemistry B 108, 827 (2004). [7] N. Dudovich, D. Oron, and Y. Silberberg, Nature 418, 512 (2002). [8] D. Pestov, R. K. Murawski, G. O. Ariunbold, X. Wang, M. C. Zhi, A. V. Sokolov, V. A. Sautenkov, Y. V. Rostovtsev, A. Dogariu, Y. Huang, et al., Science 316, 265 (2007). [9] S. Constantine, Y. Zhou, J. Morais, and L. D. Ziegler, Journal of Physical Chemistry A 101, 5456 (1997). [10] B. von Vacano, T. Buckup, and M. Motzkus, Optics Letters 31, 2495 (2006). [11] E. O. Potma, C. L. Evans, and X. S. Xie, Optics Letters 31, 241 (2006). [12] S. H. Lim, A. G. Caster, and S. R. Leone, Physical Review A 72 (2005). [13] C. C. Hayden and D. W. Chandler, Journal of Chemical Physics 103, 10465 (1995). [14] S. O. Konorov, R. F. B. Turner, and M. W. Blades, Applied Spectroscopy 61, 486 (2007). 170 \fChapter 5. Bibliography [15] A. C. Eckbreth, Applied Physics Letters 32, 421 (1978). [16] S. O. Konorov, X. G. Xu, R. F. B. Turner, M. W. Blades, J. W. Hepburn, and V. Milner, Optics Express 15, 7564 (2007). 171 \fChapter 6 Conclusion This thesis has introduced new techniques of coherent anti-Stokes Raman spectroscopy with broad band pulses: the NASCARS method, the method of optical correlation of broad band pulses, the method of complete characterization of molecular vibration and the spectral phase approach of background free CARS. These methods stress di\ufb00erent aspects of CARS and can be used under di\ufb00erent conditions. All the methods discussed in this thesis are based on the coherent property of CARS. The coherence between the vibrational levels adds correlation patterns to the noisy probe pulse, from which the vibrational resonance spacing can be extracted through spectral autocorrelation. In this way, the method of NASCARS was invented and demonstrated (chapter 2). The method of NASCARS can be implemented with collinear geometry in addition to the proof-of-principle experiment of non-collinear geometry. The single pulse version of NASCARS in collinear geometry o\ufb00ers a simple way of obtaining the vibrational level spacing of low wavenumber resonances without pulse shaping. In a broader perspective, the approach of tracking correlations within a coherent process can be an interesting topic. Considering CARS as one special type of resonant four-wave-mixing processes, possible applications of the noise correlations on general resonant four-wave-mixing can be an attractive \ufb01eld to explore. Since the method does not require exact shaping of the pulse, and noise that the light \ufb01eld gains during propagation actually helps recovering the vibration level spacing, it may have applications in the vibrational spectroscopy of high scattering media. While the NASCARS method can only recover the vibrational level spacing of the resonances, the method of optical correlation of broad band pulse is able to obtain the high resolution spectrum (chapter 3). The correlation of 172 \fChapter 6. Conclusion spectral components in a broad band pulse is now processed optically. The probe pulse of an optimized noise pattern is used to generate CARS signal and serve as an optical processing pulse in the sum frequency generation. The underlying novelty of this method is the introduction of conjugate pulse pairs. The proof-of-principle experiment was done with a pulse shaper to create a self-conjugate probe pulse. For the potential future development of this method, it would be attractive to \ufb01nd a universal way of creating a conjugate pulse for a given probe pulse and use it as a separate reference pulse. The phase-conjugate technique [1] is worth investigation. The complete characterization of molecular vibration method (chapter 4) is di\ufb00erent from the previously discussed two methods in that it stresses the recovery of maximal information from the laser induced coherent vibrations. As a result, it can not only obtain the spectrum of vibrational resonances but also the spectral phase. It achieves this complete characterization by a time-frequency two-dimensional scan. The ability to measure the phase of the vibration is the primary advantage of this method. As the experimental results demonstrate, the complete characterization approach can achieve much better spectral resolution than the probe pulse bandwidth. This is because for a coherent property, the frequency domain and time domain response are connected directly by the Fourier transform. With phase information available, the resolution on the frequency domain can be improved by increasing the range of the time domain measurement and vice versa, therefore the duration or bandwidth of the probe pulse is not a limitation. This is an e\ufb00ective solution to the \u201cresolution vs. intensity\u201d dilemma that discussed in section 1.2. Since the phase property is of central interest for coherent control, the ability to measure phase becomes a clear advantage. The direct potential application of this method would be tracking the amplitude and phase of arbitrary vibrational excitation. Since CARS is a special type of resonant four-wave-mixing, there is no reason that this complete characterization method cannot be applied to other type of resonant four-wave-mixing that may involve an electronically excited state, especially under the strong \ufb01eld condition. Due to the limited time span of my PhD study, there are other possible energy schemes (see \ufb01gure 6.1) of complete characterization 173 \fChapter 6. Conclusion of electronic excited states, which are waiting to be explored. From the perspective of data interpretation, the availability of both amplitude and phase of a coherent vibration allows a reconstruction of CARS response at any frequency or time resolution (see appendix D). In addition, this method can be used to characterize those population transfer technique such as Stimulated Raman adiabatic passage (STIRAP)[2] and the piecewise adiabatic passage technique[3]. For example, the aim of both STIRAP and piecewise adiabatic passage is to robustly transfer the complete population from the ground state to the excited via a real but not populated intermediate state through a special time ordered stimulates Raman process, that can \ufb01t into a CARS scheme (see \ufb01gure 6.2) to use the complete characterization technique of XFROG. Monitoring the amplitude and phase evolution during the STIRAP process can help optimize parameters or even improve the adiabatic passage method itself. The spectral phase approach (chapter 5) to recover the background free Raman spectrum under high non-resonant background conditions is an application of the method of complete characterization of molecular vibration. The non-resonant background is the factor that seriously limits the general application of CARS. The spectral phase approach can solve the high nonresonant background problem. The currently limitation of this approach is the overall operation time, since it involves a time delay scanning. If the time scan can be further improved by using a fast time delay device, the potential development of this spectral phase approach can be the \ufb01eld of micro-spectroscopy or even vibrational imaging of especially interested material of non-resonant background. The methods presented in this thesis are improvement on one or another aspect of CARS. With the availability of coherent broad band laser, the ability of pulse shaping and characterization, there are certainly other possibilities of improvement on CARS along those fruitful lines of research. 174 \fChapter 6. Conclusion (A) (B) W W Figure 6.1: (A) shows one variation of complete characterization scheme to a one-photon allowed electronic level, with one excitation pulse and two probing pulses (shown inside the dashed box) to obtain the spectrogram for XFROG retrieval. (B) shows a variation of complete characterization scheme to a two-photon allowed electronic level. (Probe pulse is shown in dashed box). 175 \fChapter 6. Conclusion (A) |m> Stokes Probe pump |e> |g> (B) |g> W t Figure 6.2: (A) shows the scheme of a combination of STIRAP with the complete characterization method. Two high intensity pulses transfer the population to the excited state, a weak intensity probe pulse tracks the actual transfer process in time. (B) shows the time ordering of the involved pulses. 176 \fBibliography [1] E. M. Vogel, M. J. Weber, and D. M. Krol, Physics and Chemistry of Glasses 32, 231 (1991). [2] K. Bergmann, H. Theuer, and B. W. Shore, Reviews of Modern Physics 70, 1003 (1998). [3] E. A. Shapiro, V. Milner, C. Menzel-Jones, and M. Shapiro, Physical Review Letters 99 (2007). 177 \fAppendix A MATLAB Simulation code of CARS This appendix contains simulation code in MATLAB that we used for CARS signal simulation. MATLAB is a widely used scienti\ufb01c calculation platform. It was purchased from Mathwork. We used version 7.2 for our simulation. The \ufb01rst program is to numerically generate optical pulse that can be used in subsequent CARS process simulations. A.1 Generate Pulse The program A.1 calls function shaper.m to perform pulse shaping function. A.2 Pulse Shaping The program A.2 is the content of shaper.m \ufb01le for introducing spectral phase and amplitude shaping to the numerical created pulses. A.3 CARS Process Simulation The program A.3 is the actual script that simulates the CARS process with shaped numerical pulses. The MATLAB script A.3 is capable of simulating CARS spectrum of three pulses. If one wants to simulate a single pulse CARS, a simple way is to use same pulse parameters in all three pulses, and perform proper background subtraction. For the clarity of this thesis, possible variations of this simulation script are not included in this appendix. 178 \fA.3. CARS Process Simulation Program A.1 MATLAB program that generates E \ufb01eld of a pulse function [pulsew pulset]=generate_pulse(centerw,FWHM,shaping,shapr,delay) % output pulsew and pulset are the pulse field in frequency %domain (wave number) and time domain (picosecond)input variable %centerw is the central frequency of the broad band pulse, FWHM % is the width at full width half maximum, shaping is the shaper % mask, it contains both amplitude and phase two rows e.g. % shaping=[ones(1,640);[pi*ones(1,320) zeros(1,320)]], % it also can be one row which corresponds to spectral phase only %e.g. shaping=[pi*ones(1,320) zeros(1,320)]; %it is in the shaper pixel. %shapr is the shaper number which predefined % in shaper_parameter.dat file % delay is the time delay factor in picosecond global point step; start=centerw-point*step\/2; enda=centerw+point*step\/2; z=linspace(start,enda,point); sizen=size(shaping); % the following script is to make it adaptive to amplitude %and phase or phase only shaping if sizen(1)==1 if isequal(max(shaping),min(shaping)) phasew=0;else phasew=shaper(z,shaping,shapr); end amplitude=1; else ampshaping=shaping(1,:); phaseshaping=shaping(2,:); if or(min(ampshaping)<0,max(ampshaping)>1) disp(\u2019amplitude mask out of bound.\u2019) end if isequal(max(phaseshaping),min(phaseshaping)) phasew=0;amplitude=shaper(z,ampshaping,shapr); % here it call the shaper.m function, to shaper else phasew=shaper(z,phaseshaping,shapr); amplitude=shaper(z,ampshaping,shapr); end end 179 \fA.3. CARS Process Simulation delayfactor=2*pi*z*delay\/1e12*3e10; % here the time delay is done via the linear phase shift % according to Fourier transform pulsew=amplitude.*exp(-(z-centerw).^2\/1.414\/FWHM^2) .*exp(i*(phasew+delayfactor)); pulset=fftshift(fft(fftshift(pulsew))); end Program A.2 MATLAB program that serves as pulse shaper. function phasemask=shaper(z,shaping,shapr) % shaper accept the z as a frequency array index % (in wave number) and shaping as SLM pixel % array (e.g. 128 or 640 for CRI SLM ) % The output is the spectral phase mask in the index of z global p; % global variable p is used to communicate with % the pulse shaper setting pixel=p(shapr,1);startw=p(shapr,2);pixelstep=p(shapr,3); if isequal(length(shaping),pixel)==0 disp(\u2019Shaper pixel dismatch see check shaper parameter set\u2019); % this is an error handling end pixelposition=startw+pixelstep.*(1:pixel); phasemask=interp1(pixelposition,shaping,z,\u2019nearest\u2019,0); phasemask(find(isnan(phasemask)))=0; % this line is to remove the NAN in Matlab, replace it with zero end 180 \fA.3. CARS Process Simulation Program A.3 MATLAB program that generates CARS. function [spec spwindow probet tstep]=CARS(Stokesshape,delay) % the output, spec is the CARS spectrum, spwindow is the %index array of wavenumber that corresponds to the spectrum % probet and tstep are the probe pulse in time and time step % that can be used in subsequent XFROG simulation delay is the % time delay between probe pulse and pump\/Stokes pair % Stokesshape is the pulse shaping on Stokes field, %it can be replacement with pumpshape or probeshape global point step p; global pumpcenter Stokescenter probecenter pFWHM SFWHM prFWHM; p=importdata(\u2019Shaper_parameter.dat\u2019); % Shaper_parameter.dat file in same directory storage the settings %of shaper, it is actually an array in the format %similar to shaper %calibration in my actual experiment, e.g. two pulse shapers, 128 pixel %and 640 pixel format is as follows %128.0 11604.0 14.0 %640.0 10668.0 3.0 % with pixel number starting wavenumber and pixel size spcenter=745; spband=50; %spectrometer detection window, spcenter is %the central wave length, spband is the total CCD bandwidth all in nm spwindow=linspace(spcenter-spband,spcenter+spband,2048); point=40960;step=0.5; % this is the total points in simulation, %a large number of points reduce the chance of %simulation glitch but %it also increase calculation time. tstep=1e12\/(point*step*3e10); pumpcenter=12500;pFWHM=25*16; %pump pulse central wave number and FWHM Stokescenter=1e7\/860;SFWHM=25*16; %Stokes pulse central wave number and FWHM probecenter=12500;prFWHM=20*16; %probe pulse central wave number and FWHM % % % % % the following matrix is the resonance structure the first row is the % relative resonant strength, second row is the resonant position in wave number (Raman shift) the third one is line width and the forth one is the non-resonant background number 181 \fA.3. CARS Process Simulation res=[1 0.4 0.9 0.7; 1000 1027 782 1206; 4.5 4.1 3.5 3.5; 0.005 0 0 0]; pumpshape=zeros(1,128); % this is the spectral phase mask for pump pulse probeshape=[zeros(1,64) pi*ones(1,64)]; % spectral phase shaper for probe pulse % note that here the Stokesshape is missing, because %in this script it is a input parameter [pumpw pumpt]=generate_pulse(pumpcenter,pFWHM,pumpshape,1,0); %128 pixel, 1 corresponds to the firs line on Shaper_parameter.dat %file, in my file first line is 128 pixel [Stokesw Stokest]=generate_pulse(Stokescenter,SFWHM,Stokesshape,2,0); %2 means 640 pixel SLM [probew probet]=generate_pulse(probecenter,prFWHM,probeshape,1,delay); %1 means 128 pixel SLM tscale=tstep*(-point\/2+1:point\/2); convt=pumpt.*conj(Stokest); convw=fftshift(ifft(fftshift(convt))); differencew=pumpcenter-Stokescenter; omg=linspace(differencew-point*step\/2+step, differencew+point*step\/2,point); resonance=res(1:3,:); NonR=res(4,1); Lorentzian=zeros(1,point)+ones(1,point)*NonR; %NonR is the nonresonance background for n=1:length(resonance) Lorentzian=Lorentzian+resonance(1,n) .\/(-omg+resonance(2,n)-i*resonance(3,n)); end vampw=Lorentzian.*convw; vampt=fftshift(fft(fftshift(vampw))); CARSt=vampt.*probet; CARSw=fftshift(ifft(fftshift(CARSt))); spec=CARSw.*conj(CARSw); CARScenter=probecenter+pumpcenter-Stokescenter; CARSscalewn=CARScenter+([-point\/2+1:point\/2]*step); CARSscale=1e7.\/CARSscalewn; 182 % this is to generate a spectrameter scale % that come with the CARS spectrum spec=interp1(CARSscale,spec,spwindow); %fit to spectrometer window end \fA.4. Simulation on XFROG CARS A.4 Simulation on XFROG CARS The \u201cxfrog.dat\u201d and \u201cprobe\ufb01le.txt\u201d are the output \ufb01les which are already in the required format of FROG3 software. Program A.4 MATLAB program that generates time frequency XFROG trace of CARS function output=CARSXFROG(shaping,delay) global point; [spec CARSscale probet tstep]=CARS(shaping,0); lendelay=length(delay); lenspec=length(spec); output=zeros(lendelay,lenspec); fprintf(\u2019 0%%\u2019); for nm=1:length(delay) output(nm,:)=CARS(shaping,delay(nm)); aa=fix(nm\/length(delay)*100); fprintf(\u2019\\b\\b\\b%2d%%\u2019,aa); end probet=probet(fix(point\/2)-2048:fix(point\/2)+2047); tstep=tstep*1e3; probetfilerange=[-2048:2047]*tstep; specincr=abs(CARSscale(fix(lenspec\/2)) -CARSscale(fix(lenspec\/2)+1)); speccenter=(max(CARSscale)+min(CARSscale))\/2; 183 \fA.4. Simulation on XFROG CARS prolen=length(probetfilerange); outputfile=zeros(prolen,5); outputfile(:,1)=probetfilerange\u2019; % the first column is the time index in femtosecond outputfile(:,2)=abs(probet).^2; % the second column is the total % intensity in time domain of probe pulse outputfile(:,3)=unwrap(angle(probet)); % the third column is the phase of E field outputfile(:,4)=real(probet); % the fourth column is the real part of the E field outputfile(:,5)=imag(probet); % the fourth column is the imaginary part of the E field Tincr=[delay(2)-delay(1)]*1e3; fprintf(\u2019writing files:\\n\u2019); fid = fopen(\u2019xfrog.dat\u2019, \u2019wt\u2019); fprintf(fid, \u2019%d %d %12.5f %12.5f %6f \\n\u2019, lendelay,lenspec,Tincr,specincr,speccenter); % this is the header of the XFROG trace as % the requirement of FROG3 software % lendelay is the number of delay points, % lenspec is the number of spectrameter CCD pixel , % Tincr is the time step of scanning step % specincr is the wave length increment of CCD pixel , % speccenter is the central wave length of CCD fclose(fid); save xfrog.dat output -ascii -append; fprintf(\u2019file xfrog.dat written\\n\u2019); save probefile.txt outputfile -ascii -tabs; fprintf(\u2019file probefile.txt written \\n\u2019); end 184 \fAppendix B Alignment of the Pulse Shaper and Calibration of the SLM B.1 Alignment of the Pulse Shaper A low power broad band pulse from a Ti:sapphire oscillator can help the alignment of a pulse shaper. The procedures are as follows: 1. Optical elements on table are placed as \ufb01gure B.1 shows. 2. The input mirror is adjusted to let the oscillator beam hit the grating. The light beam should pass on top of output-coupling mirror. The beam spot on grating should be at the top as \ufb01gure 1.30inset (C) dot 1 shows. 3. The grating is mounted a rotational stage. One adjusts the grating angle by rotating the stage to let the dispersed light pass above the intermediate mirror M. Figure B.1 inset (D) shows the relative position. The grating should be placed at exact vertical to the optical table. This can be checked by the dispersed elliptical light patten being parallel to the optical table. 4. The distance of the cylindrical mirror from the grating is adjusted to match the focal length. The cylindrical mirror should collimate the light to a parallel dispersed light belt. 5. The pitch of cylindrical mirror is adjusted for few degrees to make the dispersed light belt hit the intermediate mirror M at the upper part of the mirror as \ufb01gure B.1 inset (D) dot 2 shows. 6. The intermediate mirror M is set to the let the re\ufb02ected light enter 185 \fB.1. Alignment of the Pulse Shaper Back mirror A SLM Grating M Output Input Grating CM B SLM CM Input 1 1 M 2 2 Output E C 1 2 3 4 D Figure B.1: The above \ufb01gures show the setup of a folded pulse shaper. The grating on this setup is either 600 or 800groves\/mm; cylindrical mirror is f = 50cm, and CRI SLM-640 has a window size about 5cm. Figure (A) shows the top view of the pulse shaper. Figure (B) shows the side view of the pulse shaper. Insets (C) to (E) shows the light pro\ufb01le on corresponding optical elements. 186 \fB.2. SLM Voltage to Phase Calibration of CRI-SLM 640 SLM the SLM at right angle. 7. The forward\/backward and horizontal positions of the SLM are adjusted and an adjustable mirror is mounted behind the SLM to re\ufb02ect the light belt back to the bottom side of the intermediate mirror M as \ufb01gure B.1 inset (D) dot 3 shows. 8. The intermediate mirror M should re\ufb02ect the light to the cylindrical mirror. The mirror behind the SLM have to be adjusted to let the re\ufb02ected light spot on the cylindrical mirror as \ufb01gure B.1 inset (E) shows. The Light after the cylindrical mirror are re-focused onto the bottom part of grating. The grating recombines the light into uniform output beam. After the above alignment, SLM from the pulse shaper is then removed from the optical setup. The output beam is then coupled to an autocorrelator(FR103, Femtocrhome) and the distance between the cylindrical mirror and the grating is adjusted to minimize the pulse durations while monitoring the autocorrelator. After minimization of the pulse duration, the SLM should be put back to the Fourier plane and the pulse shaper optical alignment is then completed. B.2 SLM Voltage to Phase Calibration of CRI-SLM 640 SLM After the optical path alignment of a pulse shaper, the next step is to obtain the voltage vs. phase relation of the SLM. Before voltage vs. phase calibration, it is necessary to perform a quick frequency vs. pixel calibration to \ufb01nd out the frequency\/pixel correspondence. It can be done as follows: 1. The broad band pulse is aligned into the pulse shaper as appendix B.1 described 2. Arbitrary voltages are set to a serials of pixels. 3. The corresponding dips or spike on spectrum is found and related to the pixels. 4. A linear \ufb01t is performed to get the calibration coe\ufb03cient a and b 187 \fB.2. SLM Voltage to Phase Calibration of CRI-SLM 640 SLM with \u03bb = a \u00b7 n + b where \u03bb being the light wavelength and n being the pixel number. With these coe\ufb03cients obtained, the wavelength of all pixels can be easily calculated. It is used in the subsequent voltage vs. phase calibration. The fundamental idea on the voltage vs. phase calibration is to scan the voltage of the SLM pixels and measure the transmittance, and the transmittance is used to calculate the phase. A more detail description on nematic liquid crystal SLM on voltage and phase can be found in Juan M Bueno 2000 J. Opt. A: Pure Appl. Opt. 2 216-222 . An example transmittance vs. voltage curve is shown as \ufb01gure B.2 (A). A phase vs. voltage calibration \u03c6(v) (\ufb01gure B.2 (B)) can be obtained through calculation. The two masks of the CRI-SLM 640 have to be calibrated accordingly. The procedure is described as follow: 1. A pair of polarizers is placed at the input and the output of the pulse shaper. The direction of polarization on two polarizers should be set to parallel to the input beam to obtain maximal transmission. 2. The voltage value of the \ufb01rst liquid crystal layer is \ufb01xed to certain value (e.g. 1000 voltage count as de\ufb01ned by CRI) and the voltage of the second layer is scanned. 3. The spectra are recorded while the second layer voltage is scanning. The spectrum vs. voltage count is a two dimensional data array. From this array, the transmission vs. voltage curve can be extracted for each frequency. 4. The measured SLM pixel vs. frequency coe\ufb03cient is used to obtain the transmittance vs voltage curve for each SLM pixel. Figure B.2(A) shows the shape such transmittance vs voltage curve. 5. The peaks and valleys of calibration curves are located. At these locations, calibration curves are cut into segments. Within each segment, \u221a one can use the following formula \u03c6 = 2 arccos( T ) to convert transmission T into phase. 6 The segments of phase vs voltage curve are connected to get a long range, smooth phase vs. voltage curve as Figure B.2(B) shows. Because the multi-value property of arccos function, adjustment of the integer multiple of \u03c0 is required for a smooth connection of curve segments. 188 \fB.2. SLM Voltage to Phase Calibration of CRI-SLM 640 SLM Transmittance 1 (A) 0.8 0.6 0.4 0.2 0 400 600 800 1000 1200 SLM voltage count (B) SLM votage count 1100 1000 900 800 700 600 -1 0 1 2 3 Spectral phase (rad.) 4 5 6 Figure B.2: Figure (A) is the experimental recorded transmittance vs. voltage count curve (CRI SLM-640). The response between maximum and minimum locations (arrows) is used as the total transmission and null transmission to create the phase-voltage response curve shown as \ufb01gure (B). The blue curve and red in both (A) and (B) correspond to di\ufb00erent frequency component of broad band light. 189 \fB.2. SLM Voltage to Phase Calibration of CRI-SLM 640 SLM 7. The curve can be \ufb01tted using a proper continuous function (5th order polynomial was used in the experiment) to obtain the Vs (\u03c6, \u03bb) relation. After curve \ufb01tting, one should \ufb01nd the voltage value on the second layer that corresponds to zero phase shift (as calculated by the \ufb01tting function). 8. The calculated mask is then applied to the second layer. Then, the voltage value of the \ufb01rst layer and is scanned to obtain a transmittance vs voltage curve similar to that of steps 3 and 4. 9. The voltage vs. phase curve of the \ufb01rst layer is then obtained to calculate the Vp (\u03c6, \u03bb). It is similar to steps from 5 to 7. Now the calibration curves are obtained for both masks. They are used to convert the phase and amplitude values into voltage counts that can be set directly to two SLM masks. Considering that the voltage vs. phase relation is also wavelength dependent, a computer program was written to do the \ufb01tting for the range of pulse shaper light bandwidth. 190 \fAppendix C XFROG Retrieval Using FROG3 Software Due to the requirement on time and expertise on algorithm, I haven\u2019t written the XFROG retrieving script, so far FROG3 software (Version 3.2.2 ) has been used to retrieve the vibrational coherence. It was purchased from Femtosoft company (http:\/\/www.femtosoft.biz\/). FROG3 is a compiled executable program and is useful to retrieval FROG trace as well as XFROG trace in optical \ufb01eld characterization. In order to make it work in vibrational coherence characterization, the data should be organized in correct format. C.1 Obtaining and formatting the recorded data XFROG retrieval requires two sets of data. First data set is used to characterize probe pulse of the CARS. The second data set is the time-frequency CARS spectrogram (also called XFROG trace). The characterization of probe pulse can be done by FROG or MIIPS. Both intensity and phase information of the probe pulse have to be experimentally characterized. The FROG3 software is used for the actual retrieval. It only accepts data in certain format. The acceptable probe pulse format are \ufb01ve columns, comprised of time scale column, intensity column, phase column, real part column and imaginary part column. The MATLAB simulation program A.4 contains the generation of a numerical probe pulse of acceptable format. Due to the processing ability of FROG3 software, the size of numerical probe pulse is limited to 2048 points (as for FROG3 software ). Too many or too little points both reduce the FROG3 software performance and sometimes 191 \fC.2. Operation with software lead to poor algorithm convergence. The trace data should be a two-dimensional array, with row being spectrum and column representing di\ufb00erent time delay. A header \ufb01le before the data \ufb01le makes the operation with software simple. The header are an array of numbers: the \ufb01rst one is the number of delay points; the second one is the number of spectrometer CCD pixel; the third one is the time step size in femtosecond; the fourth one being the wave length increment of CCD pixel; the \ufb01fth one is the central wavelength of detection CCD. The MATLAB simulation program A.4 provides a functional sample as well. C.2 Operation with software After the installation of FROG3 software, open it and select \u201crun\u201d XFROG (hot key ctrl-x) it will bring a screen like \ufb01gure C.1 192 \fC.2. Operation with software Figure C.1: Experimentally observed time-frequency CARS spectrogram of azobenzene. (Click arrow 1 to select the XFROG (CARS) trace \ufb01le. Tick the arrow 2 box if the \ufb01le has header, if not, leave it unchecked and manually input these parameters. Select the settings to \u201cSFG\u201d for XFROG CARS at the arrow 3 position. Arrow 4 position shows the number of points, select it according to data point. A good practice for this experiment record data with points of 256,512 or 1024 points. This can avoid the subsequent interpolation. Arrow 5 and 6 positions are related to the format of trace \ufb01le. Select \u201cWavelength\u201d if in the data array row is spectrum otherwise select \u201cDelay\u201d. Select \u201cConstant wavelength\u201d if the data is recorded from a spectrometer. 193 \fC.2. Operation with software Figure C.2: After all settings correct, click \u201cOK\u201d box to go to next screen. This \ufb01gure is included as a reference. 194 \fC.2. Operation with software Figure C.3: Select \u201cRead-in E \ufb01eld from \ufb01le\u201d, then select probe \ufb01le and input the center frequency. The \ufb01le of the probe \ufb01eld \ufb01le is in time domain and should not contain fast carrier oscillation. 195 \fC.2. Operation with software Figure C.4: FROG3loads the trace and display it in logarithmic scale. For experimental recorded trace, it has some noise spot. One can use the \ufb01ve noise subtraction options to reduce noise spot.Note that the edge option potentially can change the relative ratio between highest signal and lowest signal. 196 \fC.2. Operation with software Figure C.5: One can also use the extract function to extract the region of interest. This function is used to cut the residue probe pulse. Then click the \u201cGrid data\u201d. 197 \fC.2. Operation with software Figure C.6: This screen show the experimental trace and initial guess (as a built-in function of FROG3). Click the \u201cBegin\u201d button to start retrieval. 198 \fC.2. Operation with software Figure C.7: After certain iterations, it shows convergence, which means the \u201cRetrieved\u201d two dimensional graph is the same as the input \u201coriginal\u201d spectrogram. It can be stopped or paused. If it is stopped, the retrieved E-\ufb01eld in both frequency and time domain will be saved as \ufb01le \u201cspeck.dat\u201d and \u201cEk.dat\u201d in the same folder as the trace \ufb01le. If convergence cannot be achieved, it means the input probe pulse is not accurate or the recorded two-dimensional trace has error. Due to some unknown reasons, the spectral phase of XFROG retrieval has a linear slope, this does not a\ufb00ect data interpretation. It can be trivially removed by linear \ufb01tting and subtraction. At the point where corresponding intensity is zero or close to zero, the spectral phase is also give number zero by the software. 199 \fAppendix D New Representations of Characterized Vibrational Coherence This appendix includes a submitted article to Journal of Chemical Physics by our research group with this title. D.1 Characterization of Transient Molecular Vibrations on the Way Towards Coherently Controlled Vibrational Target State Broad spectral width of ultrashort laser pulses has o\ufb00ered new possibilities for coherent control of atomic and molecular quantum states [1]. When a desired target state can be reached via multiple distinguishable paths, control can be implemented by adjusting the spectral components resonant with the corresponding interaction paths. Owing to quantum interferences, one can enhance the amplitude of the target state while suppressing others. In the case of relatively simple systems, the control \ufb01elds can be calculated a priori [2], whereas feedback controlled schemes are employed for controlling more complex systems [3]. Both approaches proved very successful in reaching the target quantum state at the end of the laser interaction with atoms or molecules. On the other hand, transient behavior, i.e. the 0 A version of this chapter is to be appeared in Journal of Chemical Physics as Stanislav O. Konorov, Xiaoji G. Xu, John. W. Hepburn and Valery Milner \u201cCharacterization of Transient Molecular Vibrations on the Way Towards Coherently Controlled Vibrational Target State\u201d 200 \fD.1. Method Content evolution of the molecular quantum state during the interaction with the control \ufb01eld, is rarely considered in the context of coherent control. Such transient dynamics may, however, become important if the intermediately populated quantum states are coupled to the irreversible decay channels, such as photo-ionization, dissociation or chemical reactions [4]. There are two reasons for the transient re-distribution of molecular population among quantum states. In addition to the \u201ccontrol\u201d resonant frequencies, continuous spectrum of an ultrashort pulse contains many o\ufb00-resonant components which induce population transfer on the time scale inversely proportional to the frequency detuning from the corresponding resonance [2]. The second reason applies to the strong-\ufb01eld regime of interaction, in which the \u201cbare\u201d eigenstates of a free-molecule Hamiltonian are signi\ufb01cantly shifted in energy during the interaction with a control \ufb01eld. Though successfully used in the strong-\ufb01eld control schemes [4, 5], these light-induced shifts may result in transient resonances leading to undesired population transfer. Here we demonstrate tracking of transient vibrational dynamics of a molecule interacting with the control laser \ufb01eld. The latter excites molecular vibration, i.e. a superposition of several vibrational eigenstates, in the ground electronic state via two-photon Raman transition (Fig.D.1). Coherent control of the target vibrational superposition state is executed by shaping the spectrum of the two-photon excitation \ufb01eld in such a way as to suppress the frequencies of certain vibrational transitions, thus leaving those vibrational modes unexcited (e.g. |b2 state in Fig.D.1). Complete time evolution of the vibrational coherence is detected by means of the cross-correlation frequency resolved optical gating of coherent anti-Stokes Raman scattering (xfrog cars [6]). We show that even though the \ufb01nal state does not include those vibrational modes whose transition frequencies were blocked in the shaped excitation \ufb01eld, these modes are strongly excited on the intermediate time scale and then de-excited at the end of the interaction. The analysis is possible due to the capability of xfrog cars to reconstruct molecular coherence with variable time and frequency resolution, without changing the experimental parameters and repeating the experiment. 201 \fD.1. Method Content Figure D.1: Energy level diagram and interaction scheme for Coherent antiStokes Raman Scattering process with spectrally shaped excitation \ufb01elds. 202 \fD.1. Method Content In the bare state basis of Fig.D.1, a wavefunction of the j-th molecule can be written as: \u03c8(rj , t) = a(t)|a + \u0002 ei(k1 \u2212k2 )rj bk (t)|bk , (D.1) k where a(t) and bk (t) are complex amplitudes of the ground and k-th excited state, respectively, for simplicity assumed identical for all molecules in the ensemble. Following the derivation of [7], it can be shown that the amplitude of the coherent anti-Stokes \ufb01eld, emitted in the phase-matching direction, is proportional to the convolution of the probe \ufb01eld amplitude and the resonant molecular response: EaS (\u03c9) \u221d Epr (\u03c9) \u2297 \u0002 k \u03c1kab (\u03a9) , \u03a9 \u2212 \u03a9k + i\u03b3k (D.2) where \u03c1kab (\u03a9) \u2261 a(\u03a9)b\u2217k (\u03a9) represents the vibrational coherence of the k-th mode, with a(\u03a9) and bk (\u03a9) being the Fourier transformed bare state amplitudes a(t) and bk (t). The xfrog cars method enables one to re-construct the complex molecular response R(\u03a9) \u2261 \u0015 k \u03c1kab (\u03a9)\/ [\u03a9 \u2212 \u03a9k + i\u03b3k ] (second term in Eq.D.2) by measuring the two-dimensional spectrogram I(\u03c9, \u03c4 ) \u2261 |EaS (\u03c9, \u03c4 )|2 , corresponding to the spectrum of the anti-Stokes \ufb01eld at variable time delays \u03c4 of the probe \ufb01eld [6]. An example of such spectrogram is shown in Fig.D.2. Two-dimensional cars spectrograms have been widely used in describing coherent molecular dynamics as they provide convenient visualization of both the spectral and temporal features of the molecular response [8, 9]. By experimentally adjusting the probe pulse duration, one can obtain spectrograms exhibiting the desired time and frequency resolution [9]. Shorter probe pulses improve the time resolution at the expense of the spectral one, while longer pulses result in the opposite e\ufb00ect. Here, we take advantage of the capability of xfrog cars to re-construct the complex-valued response function R(\u03a9) after a single two-dimensional scan. Once R(\u03a9) is determined, the molecular dynamics can be analyzed with the desired time or frequency resolution by calculating the modulus square of 203 \fD.1. Method Content Figure D.2: Experimentally obtained two-dimensial CARS spectrogram. Spectral markers around 782, 1000 and 1027 cm\u22121 indicate positions of Raman lines. 204 \fD.1. Method Content the frequency convolution \u0012 \u00122 \u02dc \u03c4 ) \u221d \u0012\u0012E\u0303pr (\u03c9) \u2297 R(\u03a9)\u0012\u0012 I(\u03c9, (D.3) with any hypothetical probe \ufb01eld E\u0303pr , yet without repeating the experiment or changing the experimental parameters of the probe pulses. Below we demonstrate this method by applying it to the analysis of coherently controlled vibrational excitation of toluene. Our cars experiments are carried out with the laser system based on a commercial Ti:Sapphire femtosecond ampli\ufb01er (40 fs, 1 kHz repetition rate) and two optical parametric ampli\ufb01ers (Fig.D.3), generating pump, Stokes and probe pulses at the central wavelength of 800 nm, 862 nm and 720 nm, respectively. In order to control the molecular vibration excited by the pump-Stokes two-photon \ufb01eld (see Fig.D.1), both pump and Stokes pulses are shaped by means of two separate spectral pulse shapers, implemented in the standard 4f geometry [10]. Placing a slit in the Fourier plane of the pump shaper, we narrow its spectral bandwidth to 3 cm\u22121 full width at half maximum (fwhm), much narrower than the frequency separation of the Raman resonances in toluene. With such narrowband pump, the spectral shape of the two-photon excitation \ufb01eld is e\ufb00ectively equivalent to the spectral shape of Stokes pulses. Control of the latter is performed by means of a double-layer spatial light modulator (SLM) in the Fourier plane of the Stokes shaper (PS1 in Fig.D.3). Both the phase and amplitude of Stokes spectrum are controlled with the resolution of 2 cm\u22121 . As shown in our earlier work [11], the robustness of the xfrog cars method can be increased by means of the spectral shaping of probe pulses. To follow that recipe, we use another pulse shaper (PS2 in Fig.D.3) and introduce a sharp phase step of \u03c0 radian in the center of probe spectrum. Pump, Stokes and probe pulses are synchronized in time and focused by means of a silver mirror (focal length of 25 cm) into a 5 mm optical path quarts cuvette with neat toluene. cars signal is spatially separated from the rest of the beams, and is coupled into a spectrometer equipped with a CCD camera and providing spectral resolution of 1.5 cm\u22121 . Two-photon spectrum of the 205 \fD.1. Method Content Figure D.3: Experimental setup. 206 \fD.1. Method Content Figure D.4: Amplitude (black) and phase (red) of the spectral shaping applied to Stokes pulses. Raman modes of toluene at 782, 1000 and 1027 cm\u22121 are indicated by dashed blue lines. 207 \fD.1. Method Content pump-Stokes excitation \ufb01eld is centered around 900 cm\u22121 and has a width of about 400 cm\u22121 fwhm. This enables us to excite three strong Raman lines of toluene at 782, 1000 and 1027 cm\u22121 . As an example of a simple control scheme of Raman excitation, we suppress the vibrational mode at 782 cm\u22121 by shaping the pump-Stokes \ufb01eld as shown in Fig.D.4. Note that instead of blocking a single spectral component at 782 cm\u22121 , we modulate the excitation spectrum periodically in such a way as to have its amplitude maximized at 1000 and 1027 cm\u22121 , and minimized at 782 cm\u22121 . Upon such shaping, Stokes pulse is split into a sequence of two transform-limited pulses separated by about 1.6 ps. We chose this shaping to make the analysis of the transient dynamics, presented below, more intuitive. Two-dimensional cars spectrogram, experimentally measured with all three incident pulses shaped as described above, is shown in Fig.D.2. Bright horizontal lines around -0.6 ps and 1 ps correspond to two transform-limited Stokes pulses separated by \u223c1.6 ps. Vertical horizontal lines around 782, 1000 and 1027 cm\u22121 are the \u201cspectral markers\u201d of Raman resonances (for more detailed interpretation of the spectrogram, see [11]). To better understand the vibrational dynamics of the system, and the mechanism behind coherent control of the Raman modes, we proceed with the xfrog retrieval of the molecular response to laser excitation [6]. In the frequency do- main, the response R(\u03a9) shows two strong lines around 1000 and 1027 cm\u22121 (Fig.D.5(a)). The resonance at 782 cm\u22121 is almost completely suppressed due to the missing spectral component at that frequency in the excitation pump-Stokes spectrum. An oscillatory pedestal can be attributed to the non-resonant cars background which reproduces the spectral shape of the pump-Stokes \ufb01eld (cf. Fig.D.4). Spectral resolution is determined by the maximum time delay between the probe and pump\/Stokes pulses. Knowledge of the spectral phase of the complex-valued R(\u03a9) makes it possible to re-construct the temporal response R(t) by means of a straightforward Fourier transform. Shown in Fig.D.5(b), the vibrational response exhibits two distinct excitation peaks corresponding to the overlap of the long pump pulse with a sequence of two transform-limited Stokes pulses. The \ufb01rst pulse excites all three Raman modes. Fast beating at the fre208 \fD.1. Method Content Figure D.5: Amplitude (black) and phase (red) of vibrational response of Toluene in the time (a) and frequency (b) domains. 209 \fD.1. Method Content quency di\ufb00erence between 782 cm\u22121 and 1000, 1027 cm\u22121 is clearly seen until the arrival of the second Stokes pulse. The latter ampli\ufb01es the vibrations at 1000 and 1027 cm\u22121 and de-excites the vibration at 782 cm\u22121 . After the second Stokes pulse, slow beating at the frequency di\ufb00erence between 1000 and 1027 cm\u22121 is well pronounced, while the fast beating with the mode at 782 cm\u22121 is signi\ufb01cantly suppressed. Here, the resolution is determined by the spectral bandwidth of the detected cars signal, rather than the duration of the probe pulse. Combining the spectral and temporal representations into a single twodimensional spectrogram often proves more informative, provided that the time and frequency resolution can be adjusted in the desired proportion. Normally, this requires repeating the experiment with a probe pulse of an appropriately chosen duration. Here, we take advantage of the availability of the complex-valued response R(\u03a9), retrieved from the experimental data as demonstrated above. We construct the required 2D spectrograms by calculating the frequency convolution (D.3) with a hypothetical transformlimited probe pulse E\u0303pr of necessary time duration, limited only by the experimentally achieved time and frequency resolution. In Fig.D.6(a), the spectrogram is calculated with the transform-limited probe pulse of 35 fs length. Fast beating between the mode at 782 cm\u22121 and those at 1000 and 1027 cm\u22121 is clearly resolved between the two Stokes pulses. After the second pulse at around 0.8 ps, fast oscillations disappear almost completely, attesting to the fact that the mode at 782 cm\u22121 has been de-excited, even though the frequency resolution is not high enough to resolve that mode spectrally. Slow beating between the resonances at 1000 and 1027 cm\u22121 , enhanced by the second excitation pulse, is clearly visible on a longer time scale. To analyze the same process with high spectral resolution, we convolve R(\u03a9) with a much longer probe pulse of 1 ps length, corresponding to the spectral bandwidth of 15 cm\u22121 (Fig.D.6(b)). This value is dictated by the time delay scanning range of the experimentally obtained cars spectrogram. Though the time resolution in this case is insu\ufb03cient to identify the sequence of two Stokes pulses, high spectral resolution provides evidence of 210 \fD.1. Method Content Figure D.6: Calculated two-dimensional cars spectrograms with high temporal (a) and spectral (b) resolution. 211 \fD.1. Method Content mode ampli\ufb01cation (bright vertical lines around 1000 and 1027 cm\u22121 ) and suppression (week vertical line around 782 cm\u22121 ). The region between -2 ps and 2 ps represents the dynamics of the system between two Stokes pulses. In summary, we demonstrate a way of tracking the vibrational dynamics of molecules with variable time and frequency resolution, after performing a single experimental scan of coherent anti-Stokes scattering. The method is based on the xfrog retrieval of the complex-valued vibrational response function. We show the ability to analyze the mechanism behind coherent control of the vibrational response of toluene with shaped excitation pulses. Evolution of the molecular coherence can be followed and interpreted on di\ufb00erent time scales and with correspondingly di\ufb00erent spectral resolution, yet without repeating the experiment or changing experimental parameters. 212 \fBibliography [1] M. Shapiro and P. Brumer, Principles of the Quantum Control of Molecular Processes (Wiley, New York, 2003). [2] N. Dudovich, D. Oron, and Y. Silberberg, Nature 418, 512 (2002). [3] A. Assion, T. 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Milner, Optics Express 15, 7564 (2007). 213 ","type":"literal","lang":"en"}],"http:\/\/www.europeana.eu\/schemas\/edm\/hasType":[{"value":"Thesis\/Dissertation","type":"literal","lang":"en"}],"http:\/\/vivoweb.org\/ontology\/core#dateIssued":[{"value":"2009-11","type":"literal","lang":"en"}],"http:\/\/www.europeana.eu\/schemas\/edm\/isShownAt":[{"value":"10.14288\/1.0061624","type":"literal","lang":"en"}],"http:\/\/purl.org\/dc\/terms\/language":[{"value":"eng","type":"literal","lang":"en"}],"https:\/\/open.library.ubc.ca\/terms#degreeDiscipline":[{"value":"Chemistry","type":"literal","lang":"en"}],"http:\/\/www.europeana.eu\/schemas\/edm\/provider":[{"value":"Vancouver : University of British Columbia Library","type":"literal","lang":"en"}],"http:\/\/purl.org\/dc\/terms\/publisher":[{"value":"University of British Columbia","type":"literal","lang":"en"}],"http:\/\/purl.org\/dc\/terms\/rights":[{"value":"Attribution-NonCommercial-NoDerivatives 4.0 International","type":"literal","lang":"en"}],"https:\/\/open.library.ubc.ca\/terms#rightsURI":[{"value":"http:\/\/creativecommons.org\/licenses\/by-nc-nd\/4.0\/","type":"literal","lang":"en"}],"https:\/\/open.library.ubc.ca\/terms#scholarLevel":[{"value":"Graduate","type":"literal","lang":"en"}],"http:\/\/purl.org\/dc\/terms\/title":[{"value":"New methods of coherent anti-Stokes Raman spectroscopy based on broadband pulses","type":"literal","lang":"en"}],"http:\/\/purl.org\/dc\/terms\/type":[{"value":"Text","type":"literal","lang":"en"}],"https:\/\/open.library.ubc.ca\/terms#identifierURI":[{"value":"http:\/\/hdl.handle.net\/2429\/8445","type":"literal","lang":"en"}]}}