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Mathematical modelling of the combined effects of vortex-induced vibration and galloping Corless, Robert Malcolm 1986

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Mathematical Modelling of the Combined Effects of Vortex-Induced Vibration and Galloping By Robert Malcolm Corless B.Sc, The University of British Columbia., 1980 M.Math., The University of Waterloo, 1982 A THESIS S U B M I T T E D IN PARTIAL F U L F I L L M E N T O F T H E R E Q U I R E M E N T S FOR T H E D E G R E E O F D O C T O R O F PHILOSOPHY in T H E F A C U L T Y O F G R A D U A T E STUDIES Department of Mechanical Engineering We accept this thesis as conforming to the required standard T H E UNIVERSITY OF BRITISH COLUMBIA November 1986 © Robert Malcolm Corless, 1986 In presenting this thesis in partial fulfilment of the requirements for an advanced degree at the University of British Columbia, I agree that the Library shall make it freely available for reference and study. I further agree that permission for extensive copying of this thesis for scholarly purposes may be granted by the head of my department or by his or her representatives. It is understood that copying or publication of this thesis for financial gain shall not be allowed without my written permission. Department The University of British Columbia 1956 Main Mall Vancouver, Canada V6T 1Y3 Date March 3o, mi DE-6(3/81) A b s t r a c t In this thesis a mathematical model for the combined effects of vortex-induced oscillation and galloping of a square section cylinder in cross flow is examined. The model equations are obtained by simply combining Parkinson and Smith's Quasi-Steady Model for galloping with the Hartlen-Currie model for vortex-induced vi-bration, which is essentially the same model used by Bouclin in the hydrodynamic case. The semi-empirical model is solved using three popular approximate analyt-ical methods, and the methods of solution are evaluated. The solution of the model is compared with recent experimental data. The methods of solution used are the Method of Van Der Pol, (also called the method of Harmonic Balance), the Method of Multiple Scales, and some results from the Hopf Bifurcation Theory. The Method of Multiple Scales provides the most useful solutions, getting good results even with just the 0(1) terms, although the next-order terms are necessary for the solution in the resonance regions. The phenomenon of subharmonic resonance, observed in recent experiments, is also observed in the solution of the model equations. ii Contents Abstract ii List of Figures v Nomenclature vi Acknowledgements ix 1. Introduction 1 1.1 Outline of the Problem 1 1.2 Vortex-Induced Vibration 4 1.3 Galloping 6 1.4 Interaction Effects 7 2. Proposed Mathematical Model 10 2.1 General Remarks 10 2.2 Functional Form of the Parameters 16 3. Model Synthesis 20 3.1 Parameters Fixed by Static Experiments 20 3.2 Experimental Determination of a, B, and D 22 4. Methods of Solution of the Model Equations 25 4.1 Discussion of Available Methods 25 5. Solution by the Method of Van Der Pol 33 5.1 Setting up the Equations 33 5.2 Solution of the Polynomial Equations 35 5.3 Results of the Method of Van Der Pol 37 6. Hopf Bifurcations of the Model Equations 43 6.1 Introduction 43 6.2 Hopf Bifurcation Theory 44 6.1 Bifurcation Formulae 46 iii 6.4 Bifurcation of the Quasi-Steady Model . 50 6.5 Limitations of the Hopf Bifurcation Theory 54 6.6 Model Equations 55 6.7 Location of the Hopf Bifurcation Points 55 6.8 Coefficients of the Bifurcation Polynomial 58 6.9 Results of Bifurcation Formulae 61 7. Solution by the Method of Multiple Scales 71 7.1 Overview and Choice of Time Scales 71 7.2 Case I: Resonance Case, with UJQ = 1 + //wi 75 7.3 Solution of the O(n) equations 79 7.4 Stability of the 0(/u) solutions 81 7.5 Solution to 0{fi2) 83 7.6 Case II: Nonresonance Case, with u>o 76 1 95 7.7 Nonresonance Solution to O(fi) 108 7.8 Subharmonic Solution to O(fx): UIQ = 3 + ^ 3 112 7.9 Superharmonic Solution to O(fi) 120 7.10 Results of the Method of Multiple Scales 130 8. Comparison with Experiment 146 8.1 Concordiat of Solutions 146 8.2 Behaviour in the Quasi-Steady Limit 150 8.3 Comparison of Predictions 152 9. Conclusions 156 9.1 Conclusions 156 9.2 Suggestions for Further Work 159 IV List of Figures 1.3.1 Equivalent Angle of Attack 8 3.1.1 Polynomial Force Coefficients 21 5.3.1 Van Der Pol Solution Amplitude 41 5.3.2 Van Der Pol Solution Excitation 42 6.4.1 Quasi-Steady Bifurcation 53 6.9.1 Hopf Bifurcation Points 66 6.9.2 Hopf Bifurcation for larger n 67 6.9.3 Hopf Solution for Low Damping 68 6.9.4 Hopf Solution for Medium Damping 69 6.9.5 Hopf Solution for High Damping 70 7.5.1 Solution in the Resonance Region 94 7.6.1 Steady State Amplitudes /'(0) > 0 106 7.6.2 Steady State Amplitudes /'(0) < 0 107 7.6.3 Solution to O(l) 109 7.10.1 Low Turbulence Amplitudes 137 7.10.2 Low Turbulence Excitation 138 7.10.3 Medium Turbulence Amplitudes 139 7.10.4 Medium Turbulence Excitation 140 7.10.5 High Turbulence Amplitudes 141 7.10.6 High Turbulence Excitation 142 7.10.7 Amplitude with Subharmonic Resonance 143 7.10.8 Hydrodynamic Amplitude 144 7.10.9 Hydrodynamic Excitation 145 8.1.1 Ui versus U0 151 V Nomenclature A 0 - Complex amplitude of the O(l) oscillation for the method of multiple scales. Al - Complex amplitude of the 0(p) oscillation for the method of multiple scales. A 2 ~ Complex amplitude of the 0(p2) oscillation for the method of multiple scales. ao — Real amplitude of the 0(1) oscillation for the method of multiple scales. ai — Real amplitude of the O(n) oscillation for the method of multiple scales. a 2 — Real amplitude of the 0(p?) oscillation for the method of multiple scales. a(wo) — Van Der Pol (Rayleigh) equation coefficient. Ak- Polynomial fit coefficients from the quasi-steady theory, k = 1, 3, 5, • • •, N. B — Acceleration coupling coefficient from the model equations. B 0 - Complex amplitude of the 0(1) excitation for the method of multiple scales. S i - Complex amplitude of the O(fx) excitation for the method of multiple scales. 6 0 - Real amplitude of the 0(1) excitation for the method of multiple scales. bi - Real amplitude of the O(p) excitation for the method of multiple scales. JP Lateral force coefficient, = —^—. cv - Nondimensional excitation coefficient. Fixed cylinder excitation amplitude. C 0 - O(l) term of Cv used in the method of multiple scales. Cx - O(n) term of Cv used in the method of multiple scales. D — Velocity coupling coefficient from the model equations. f - vortex formation frequency from one shear layer. f(ao) - Polynomial in ao whose roots are the steady-state amplitudes to first order. Lateral aerodynamic force per unit cylinder span 9 — The Van Der Pol coefficient a(wo) in asymptotic form for the method of multiple scales: fig — a(uo). h — Width of cylinder cross section Coefficient of eikT in Y2, k = 3, 5, 9. m — Mass of cylinder per unit span. n — Mass ratio 2m Tfc — Quasi-steady polynomial coefficients in asymptotic form: /x2r^ = nU2Ak/Uk for k = 3,5,7 and p2rx — n(U -U0)A\. 5 — Model coupling coefficient in asymptotic form, /z2s = ret/2. vi S — Strouhal number, = fh/V. t — Time, nondimensionalized so the natural frequency of oscillation of the cylinder is 1, t — wxnatural time. T — Time with detuning parameters added, T = Qt. U — Nondimensional wind speed, U = Ui/Ur — Alternate notation for W{. UQ — Critical reduced wind speed for galloping from the quasi-steady theory, Ur — Reduced wind speed for vortex resonance, Ur = l/(2nS). V — Wind speed. W0 — Ratio of U0 to Ur, or 4nS/3/nAx. Y — Nondimensional displacement of cylinder during oscillation, Y — y/h. y — Displacement of cylinder during oscillation. y — Vibration velocity. a — Van Der Pol coefficient, in the special case a(u>o) = ftwo-/? — Fraction of critical viscous system damping. 7 — Van Der Pol coefficient in asymptotic form, fi^j = g ^ ^ l . S — Limit cycle TX -frequency. Ki — Coefficient of etT in Cx. K 3 — Coefficient of et3T in Cx. *C3w„ — Coefficient of e i ( 3 u ° ) T in Cx. *2u»„ + i — Coefficient of e*"(2<*>+i)r in Cx. K 2 W o - i — Coefficient of ei(*"o-i)T M C I K W o + 2 — Coefficient of e*'(<"o+2)T j n QX. « w 0 - 2 — Coefficient of e ^ u ° - ^ T in Cx. A — A convenient parameter for calculations, A = i(iD — B)AQI(U>Q — 1). H — An asymptotic parameter, arranged for the method of multiple scales so that /j,2 — n and p, a a(u;o). v — A convenient parameter for calculations, v = iu>oBo-£1 — Phase difference in the resonance region, f 1 = (f>x — ipo-£2 — Phase difference in the resonance region, £2 = 4>2 ~~ V'l-p — Fluid density. <7fc — Detuning parameters in fl, fl = 1 -+- p.ox + /x2o*2 + • • •. Tk — Slow time scales, r^  = fikT, k — 1,2,3,4. vii (Po — Phase angle of O(l) coefficient of e l T in Yo, set to zero by freedom of choice of origin. <j)\ — Phase angle of O(fi) coefficient of e'T in Yj. <p2 — Phase angle of 0(//2) coefficient of elT in y2. ibo — Phase angle of O(l) coefficient of elu),lT in Co-tpi — Phase angle of O(p) coefficient of eluJ,,T in Cj. to — Natural circular frequency of oscillation of cylinder, wo — Nondimensional wind speed (Strouhal Frequency) UQ = U/Ur. U{ — Hopf Bifurcation Point. f) — Detuning, fl = 1 + Mfco"fc-viii Acknowledgements I would like to thank most of all my wife Sumaya, for her truly loving support, encouragement, sympathy, and patience. Next I would like to thank my supervi-sor, Dr. G. V. Parkinson, for his continuing interest and useful suggestions. Also, members of my supervisory committee, in particular Dr. I. S. Gartshore and Dr. B. Seymour, raised points of interest and gave valuable suggestions. David Hare provided assistance with TeX, writing many of the macros used to produce this the-sis. I also thank the Natural Science and Engineering Research Council of Canada for their generous support, and the Departments of Mechanical Engineering and Mathematics for the support offered in the form of assistantships. Lastly, I thank my parents, and my parents-in-law, for their extreme generosity and confidence; without them, this thesis would never have been possible. C h a p t e r 1 Introduction So high they stood, that they might have been clouds in the upper air; save that they swam not as clouds, but persisted, and that their architecture was not cloud-like, but steadfast, as of buildings of the ancient earth; ... and yet all as if of no gross substance, but rather thin spirit ... —E. R. Eddison. 1.1 O u t l i n e of the P r o b l e m The problem of flow-induced vibration of two-dimensional cylinders of various cross-sections has a long history of study, arising from the discovery, in the last half century, that the aeroelastic effects of wind on structures can be as important as the effects of steady wind loads. Some of these observed aeroelastic effects are the result of coherent interaction of the wind with the structure, and should be distinguished from the response of structures to the random effects of the turbulence present in natural winds. We will consider here two of these coherent forms. l Chapter 1: Introduction 2 The commonest of these is that caused by the organized wake vortex sys-tem. Downstream of an aerodynamically bluff body, a separated wake forms, with breadth approximately that of the body. The separating shear layers are unstable, and roll up to form discrete vortices. Under relatively two-dimensional conditions, the vortices are swept downstream and form two parallel rows with equal vortex spacing, staggered so the vortices alternate. For a particular structure, it is ob-served that the vortices in each row form at a frequency / proportional to the incident wind speed V and inversely proportional to the diameter h of the body. The proportionality constant is the Strouhal number This number is typically about 0.2 for cylinders of moderately symmetrical cross section. Because of the alternating pressure loading on the structure caused by this organized wake vortex system, the structure is subject to a periodic forcing, at frequency / in the direction transverse to that of the flow, and to a weaker drag force with frequency 2/, acting in the direction of the flow. If the natural frequency of the body is near these frequencies, one can expect the structure to develop a resonant response. The response of course depends on the natural mode corresponding to the natural frequency, but as is usual in any problem the simplest responses occur Chapter 1: Introduction 3 the most often. Here we will only be considering strictly transverse oscillation of a cylinder of square cross section under two-dimensional conditions. The Strouhal number for this cylinder is 0.13. . The other important coherent form of wind-induced oscillation that we will be investigating is called galloping. Galloping is a low-frequency, high-amplitude os-cillation due to a classical instability in which the body, experiencing a bump in a direction normal to the wind, receives a further aerodynamic force in the direc-tion of the bump, tending to increase the motion. This class of oscillations occurs for the same types of structures as vortex-induced oscillations, but requires some asymmetry, so that a cylinder of circular cross-section will not undergo galloping, but a square cylinder will. The final catastrophic oscillation of the original Tacoma Narrows Suspension Bridge in 1940 was an example of torsional galloping. Trans-mission lines, normally too symmetrical to gallop, can become covered in ice on one side, giving enough asymmetry to gallop and ultimately break. The stall flutter of an airfoil about its stalling angle is also an example of galloping. The interest in the interaction of the two forms of oscillation, possible under certain conditions, arises from the fact that modern tall buildings are more lightly constructed for reasons of economy than previously, and the trend in design is more toward conditions where both forms of oscillation can occur. Sullivan [24] has noted experimentally that for some reasonable parameters the observed amplitude of os-Chapter 1: Introduction 4 cillation of a three dimensional model of a tower of square section in a wind tunnel simulation of the natural wind is greater than that expected from considerations of either form of oscillation alone. Further experiments by Wawzonek [26] indicated that this interaction also occurs in the case of a cylinder of square cross-section un-der two-dimensional flow conditions. Recent experiments by Bearman, Gartshore, Maull, and Parkinson [l] (hereafter referred to as BGMP) have confirmed this by more detailed study, including wake frequency measurements. A separate, hydro-dynamic, study was earlier carried out by Bouclin [5], showing some significant interaction in the case of oscillation in water, also. 1.2 Vortex-Induced Vibrat ion Vortex-induced vibrations can occur for any aero dynamically bluff cylinder with an appreciable afterbody. The afterbody, downstream of the separation points, interacts with the wake system to give rise to the pressure loading on the body. Most studies of vortex-induced vibration have been carried out on the circular cylinder, which does not undergo galloping, but a square cylinder will undergo both forms of flow-induced vibration. Most of the qualitative phenomena associated with vortex-induced vibration are the same for both the square and the circular cylinder, and so the discussion which follows applies to both. The phenomena which occur have been experimentally observed by many, in-Chapter 1: Introduction 5 eluding Feng [8]. Vortex-induced vibrations characteristically are limited in am-plitude to the order of magnitude of one cylinder diameter, and occur only in a discrete range of windspeeds. Nondimensionalizing time so that the natural fre-quency of oscillation of the body is 1, we have by the Strouhal relationship that the wake frequency of a stationary cylinder is 1 when the nondimensional wind speed U = Ur — l/(2nS), or equivalently when the Strouhal frequency u>0 = U/Ur = 1. One would expect that the maximum amplitude of vortex-induced oscillation would occur at this wind speed, but such is not in fact the case. Nonzero amplitudes of oscillation begin for COQ just less than 1, and continue for a range of w 0 typically up to about 1.5, and the maximum amplitude occurs at about UIQ = 1.3. The frequen-cies measured in the wake in this wind speed range do not contain the expected Strouhal frequency, but rather just a frequency very close to the natural frequency of the body. The body is of course oscillating at this frequency. This is the phe-nomenon of synchronization, or lock-in. It is also possible to have a hysteresis effect, where there are two different possible stable amplitudes of oscillation at the same wind speed. Different structures under three-dimensional conditions will have different quan-titative behaviour. Most importantly, there will be several natural frequencies cor-responding to different modes of oscillation, and these will correspond to different ranges of the wind speed at which vortex-induced oscillation can occur. The sys-Chapter 1: Introduction 6 tern damping is an important parameter, and increasing the damping will naturally decrease the amplitude of oscillation. However, decreasing the system damping will only increase the amplitude of oscillation until the maximum amplitude is on the order of one diameter, as this form of flow-induced oscillation is self-limiting. 1.3 Galloping Galloping occurs, as with vortex-induced oscillation, at the natural frequency of the body. The principal qualitative differences between vortex-induced oscillation and galloping are, first, that galloping occurs typically for all wind speeds above a critical wind speed UQ that depends on the system damping, the mass, and the aerodynamic shape of the structure, whereas vortex-induced oscillations occur only in a discrete range, and second, that the amplitudes occurring in galloping oscilla-tions are very much larger, having been observed to be as much as 100 times the diameter of the structure for some ice-covered transmission lines. It is important to note that the smaller size of the vortex-induced oscillations mitigates their effect somewhat, but under certain conditions can have just as deleterious an effect on a structure as a larger amplitude oscillation through fatigue of the materials involved. For an aerodynamically bluff shape with fixed separation points, such as a square cylinder, the shear layers separating from the body can be considered symmetrical. In fact, of course, the vortex-induced fluctuations of the shear layers are also present, Chapter 1: Introduction 7 but under certain conditions we can consider only the time-averaged placement of the shear layers. If the frequency of vortex shedding is sufficiently different from the natural frequency of oscillation of the body, then the important criterion for the force on the body is the placement of the time-averaged shear layers. This observation is what we would expect from a linear theory, but, as we have already noted in the case of vortex-induced oscillation, the linear theory is often misleading. However, this observation is justified when VQ ~> UT by the success of the quasi-steady theory, which is based on this assumption and the assumption that the force felt on the cylinder in motion is the same as that felt on a stationary cylinder held at the equivalent angle of attack a. When the cylinder undergoes a motion in the transverse direction, the vector sum of the velocity of motion of the body and that of the wind gives rise to a wind at an apparent angle of attack a, where tan(a) = y/V — Y/U (see Figure 1.3.1). The quasi-steady assumption is that the force on the body resulting from this apparent angle of attack is the same as that measured on a stationary cylinder mounted at that angle of attack. Thus measurements of this simpler kind give information that we can use to predict the dynamic response of the cylinder. More detailed discussion of this follows in Chapter 2. Chapter 1: Introduction 8 average sV\eo.r /acjer V ^ / /////////////ty I I / / / / / / / / / / / / / / A Figure 1.3.1 Equivalence of a transverse perturbation and a wind at a nonzero angle of attack a. 1.4 Interaction Effects When the vortex-shedding frequency is near the body frequency, the assumption that the time-averaged shear layer shape is the most important determining feature of the motion of the body is violated. Thus one would expect that the quasi-steady theory developed for galloping would no longer apply, as it is the periodic disturbances of these shear layers, averaged out for the quasi-steady theory, which play the largest role in the motion of the body. Here we expect the theory of vortex-induced vibration to play the largest role, and under most circumstances it does. Chapter 1: Introduction 9 However, it is possible that the phenomena underlying the quasi-steady theory will play a role in this region, as well. Significant interaction effects'have in fact been observed by Sullivan [24], Waw-zonek [26], and most recently by BGMP [1]. They found experimentally that when U0 ^> UR, that is, when U0 ss UR or U0 < UR, that galloping and vortex-induced vibration appeared to interact, making the theories for each individual case not as useful. In fact, the experiments indicated in the case U0 w UR that the observed amplitudes were significantly higher than those predicted for either form of vibra-tion alone. When instead UQ < UR, they found that galloping began not at U0 as predicted by the quasi-steady theory, but rather at UR. This appears to be a result of a quenching effect of the vortex system on the galloping instability, which holds until the vortex system itself begins to move the cylinder, at which wind speed the system begins to gallop. Also, a small but significant apparent subharmonic resonance was detected by BGMP, strongly associated with a peak in the wake excitation at a frequency three times the natural frequency of the body. It is desired to develop a theory which will explain all of these effects, and retain the predictive capability for the case of galloping and vortex-induced vibration taken separately. Chapter 2 Proposed Mathematical Model 'So we be at one as for the end,' replied Beroald, 'it should be no unexampled dif-ficulty to find out the means.' — E. R. Eddison 2.1 General Remarks We are looking for a semi-empirical model of the combined effects of vortex-induced vibration and galloping. This means that we would like a mathematical model with a few free parameters that can be fixed by simple experiments; sim-ple, that is, in comparison with the full dynamic investigations done in, e.g., [l]. Where possible, we would like the parameters to be fixed by experiments on a static cylinder, and thus depend only on the geometry. For simple galloping, this goal is achieved; Parkinson and Smith's quasi-steady model [20] is very accurate, given only the polynomial fit of Cy versus tan(a) data from the fixed cylinder, in the case that U0 » Ur. For vortex-induced vibration, however, the Hartlen-Currie model 10 Chapter 2: Proposed Model 11 [10], requires that some forced-vibration experiments be done to fix some of the parameters, if they are not to be chosen ad hoc. We expect that for full agreement with the experimental data over a wide range of wind speeds that we shall have to do the same here. Note that a fully rational model would enable us to predict the dynamic behaviour when only the geometry is known; naturally, such a model would in this case be very complicated. With the present semi-empirical approach, we hope to avoid some of the complexity, while retaining the predictive character-istics: from the results of simple experiments, we hope to predict the results of complicated experiments. Parkinson and Smith's Quasi-Steady M o d e l [20]. The first model that we shall make use of is Parkinson and Smith's quasi-steady model of galloping. We model the displacement of the cylinder with the following equation: pV2 y + 2{3y + y = -—CF  y y y 2m w which we nondimensionalize to Y + 2(3Y + Y = nU2CFii. The forcing term on the right hand side is determined by the fluid mechanics of the system, and is modelled here by the use of the quasi-steady assumption. We saw earlier that the force on a cylinder at an angle of attack a can be measured Chapter 2: Proposed Model 12 relatively easily; by the quasi-steady assumption, this can be taken to be the force on a cylinder moving transverse to the wind with velocity Y, where the correspondence is given by tan (a) = Y /U. We fit a polynomial in tan (a) to the measured data, and use this expression as a polynomial in Y/U in the above equation. The linear derivative term is of particular importance, and we include the system damping here by putting which gives, redefining Cp to include this damping term, Y + Y.= nU2CFy where now This is a single degree of freedom nonlinear oscillator system. It can be solved analytically by many approximate methods when the mass parameter n is small enough, as it is in the case of aerodynamic oscillation, and may also be in some hydrodynamic cases. Parkinson and Smith used the method of Krylov-Bogoliubov to solve this equation, with very good results when t/0, the above calculated critical wind speed, was much larger than Ur. In particular, all the qualitative features of galloping discussed previously were reproduced by the solution to this model, and Chapter 2: Proposed Model 13 the quantitative accuracy of the solution is also of a high order of accuracy. Certain features of the solution are easy to see without much analysis. It is obvious that Y = 0 is a solution of the equations, and its stability is obtained by considering the equation linearized about 0. But this is just a linear oscillator, with damping proportional to — (1 — U0/U). Thus the damping is positive if U < <70, and hence the zero solution is stable. If on the other hand U > UQ then the damping is negative, and the zero solution is unstable. This corresponds precisely with the observed characteristic of galloping, that galloping occurs only for winds above a certain critical wind speed. This observation is in fact independent of the size of n, which the approximate analytical solutions generally require to be small. A more complete solution, however, is required to determine the large-amplitude behaviour of this oscillator. This was done in [20], and the solution compared to experimental data. The solution included a hysteresis loop, and the mathematical solution showing this corresponded well with the experimental data. T h e H a r t l e n - C u r r i e M o d e l [10]. In the case of vortex-induced vibration, no complete theory exists. However, the Hartlen-Currie model achieves a good qualitative agreement with experiment, and some reasonable quantitative accuracy. With this theory, we start with the same Chapter 2: Proposed Model equation as for the galloping theory, 14 Y + 2/3Y + Y = nU2Cv but now the right hand side is chosen for agreement with the qualitative features of vortex-induced vibration. First, it is desired that the right-hand side reflect the periodic nature of the excitation. Next, we note that for a stationary cylinder, the excitation on the cylinder due to the wake system is self-starting and self-limiting with a limiting amplitude of Cy(), typically on the order of 1 (we have nondimensionalized so the cylinder diameter is l). This suggests the following nonlinear oscillator equation for Cv: Cv + ulCv = au0 (dv - ~^-^C*) + DY. This is the simplest equation giving the desired qualitative properties, and, coupled with the DY term to the first equation, simply models the effect of the vortex system on the body. Here, a and D are essentially free parameters, to be chosen to make the solution fit the experimental data. Proposed Mathematica l M o d e l . Bouclin [5] took the mathematically natural approach of simply adding Cpy and Cv for investigation of hydrodynamic oscillation. He also changed the functional form of auo, making it a constant, which he called GCYo, for unstated reasons. Chapter 2: Proposed Model 15 We shall pursue this model further, examining some generalizations, and ultimately providing a useful approximate solution, instead of the numerical solution used by Bouclin in the hydrodynamic case. Our proposed model is only slightly generalized from his: (2.1.1) Y + Y = nU2{CFy + Cv) (2.1.2) Cv + w2Cv = a{u0) [Cv - * 2 C v 3 ) + D{u0)Y + B(to0)Y where CFy is as in the quasi-steady model (including /3) and C„ is as in the Hartlen-Currie Model. The only new term is the BY coupling term in the second equation, added as it is reasonable to expect some effects of the cylinder acceleration on the wake vortices. The dependence of the parameters a, B, and D on the wind speed u0 is also explicitly noted. Remark Note that we take only the simplest linear combination of the two forms. Adding another parameter, A say, making CFy + A C„, instead of CFy + Cv, can be shown to be redundant, as a scaling of the other parameters (Cy(l in partic-ular) can be used to make A = 1. Remark This model differs little from that used by Bouclin, aside from the new term B((JJQ)Y. The main thrust of this thesis will be to show that there is a useful approximate analytical solution to these model equations, and to discuss the effect Chapter 2: Proposed Model 16 of the functional dependence of the parameters on the solution. There are further natural generalizations to make; for example, adding a Cv term to equation (2.1.1), or adding more nonlinearities to. equation (2.1.2). Further nonlinearities could be added to the first equation, but these would be equivalent to changes in the second equation. We pursue the simple approach here, proceeding to complicated forms only if it proves to be necessary. 2.2 Functional Form of the Free Parameters Of the parameters in equations (2,1.1)—(2.1.2), all are determined by exper-iments on a fixed cylinder, except /?, a(u/o), B(uo), and D(UQ). The damping /? can be determined independently of the wind speed, by still-air measurements. The parameters Cy u and Ak [h = 1, 3, 5, 7) are assumed constant. This assumption seems valid for the Ak, but is not strictly true for Cy 0 , although it is good enough for our purposes here. The other parameters, though, are completely unspecified. Clearly by choosing the functional dependence correctly, we may fit any specified dynamic data, in an ad hoc fashion. However, this is contrary to the philosophy of the semi-empirical approach. We wish to have a simple functional form for the free parameters, with as few constants to be measured as necessary. In this section we explore some mathematical suggestions for the functional form of these parameters. Chapter 2: Proposed Model 17 Hartlen and Currie [10] take a(u;0) = « W Q , to make the logarithmic increment 6 = 7ra(u>o)/2uo independent of w0, and hence constant for small changes in the Reynolds number. Bouclin [5], however, takes a(u>o) = CCy n to be constant, for unstated reasons. As he obtained quite reasonable results, except perhaps for over-predicting the amplitude near wo = 1/3, this may be justified, but we are interested in making a definite choice. To look at this closer, we look at the equation (2.1.2) in the simple case when B = 0 and D = 0, corresponding to a fixed cylinder. Making the change of variable s = u)0t, C = C„/Cy„, and denoting a(u)0)/ujo by e, we have (2.2.1) C"-e{C- -(C') 3) + C = 0 3 where C = ^f-. Note that e = a in the Hartlen-Currie case, while for Bouclin as ' e = GCyo/u>0. Now (2.2.1) is a Rayleigh equation (also sometimes called a Van Der Pol equation, because they are equivalent), whose solution is well understood. For small e, the solution approaches a near-circular limit cycle of radius « 1. For large e, the solution approaches a nearly-discontinuous limit cycle, which has very sharp corners in it. Thus for moderately large e we expect the solution to depart from a purely harmonic condition and acquire significant higher-frequency components. For this equation we do not have any even-frequency components, so the next most important frequency is 3 (corresponding to 3u>o on the i-scale). Thus if a and GCYo are equal at resonance (uo — 1), near wo = 1/3 we have e three times larger in Bouclin's case than in the Hartlen-Currie case. The larger e implies a larger Chapter 2: Proposed Model r 18 component at the higher frequency, which implies a larger superharmonic resonance in the full model. This argument is of course not meant to be rigorous, but rather to suggest that the Hartlen-Currie model is superior in this respect. Later we will see that other functional forms for a(u>o) are useful, and do not suffer from this defect. For D(UQ), we look at the physical model. The original model of Hartlen-Currie used a constant, for simplicity. However, when one looks at the model, one really expects the important coupling value to be not the velocity of the cylinder, but the ratio of the velocity of the cylinder to the fluid velocity. Thus we expect that the functional form of D(u>o) to be D(u0) = —. We will see later that the solution of the model equations agrees better in the limit as U0 > UR. Lastly, we look at the coefficient B(U)Q). It is not easy to find suggestions as to the form of this coefficient, except perhaps from the model equation itself. If we look at the quasi-steady equation, we have Y Y and CFU is seen to be composed of terms that depend only on the ratio Y/U. If Chapter 2: Proposed Model 19 the relevant parameter for the velocity coupling is Y/UJ0 (equivalent to Y/U), then we might try Y/U2, and thus be led to a functional form „ , . B B(u0) = ~2. We find, however, that with this form we cannot get a significant subharmonic res-onant response. To exhibit a significant subharmonic response, we use the following ad hoc functional form for B, B{UJ0) = B0 + B2u2, and choose the parameters BQ and B2 to give the right qualitative subharmonic response. Chapter 3 Model Synthesis / hope you will wisely think you before-hand, using meditations and weighings pro and contra, afore you begin... —E. R. Eddison 3.1 Parameters Fixed by Static Experiments The coefficients A\, A3, As, and A7 are fixed in the usual fashion by measuring the force on a static cylinder at different angles of attack. The main source of differences in the non-dimensional coefficients seems to be in the turbulence levels. Later, we will be comparing the approximate analytical solutions with data taken from [l], so we will use their lateral force coefficient data to find the Ak- The experiments reported in [l] were done at three different turbulence intensities, and thus we must do three different polynomial fits [Fig. 3.1.1]. Remark It is of course a 'kitchen' problem to fit a polynomial to data, but we note here that in order to secure agreement between the A\ coefficient reported 20 Chapter 3: Model Synthesis 21 Figure 3.1.1 Lateral Force Coefficients from [1] for varying turbulence levels v'/V Data Polynomial Fit 0.0% A — 4.87* - 421*3 + 17000*5 - 194000*7 6.5% X 3.95* - 51.4*3 10.5% • — 3.15* -47.1*3 where * = tan (a). in [l] and that found with the least-squares fit, it was necessary to use a weighted least-squares fit. This was done because it is important to secure good values for Ai, as the model is quite sensitive to this value. For the medium and high-turbulence case, since we were fitting a cubic rather than a 7tfe-degree polynomial, it was easier to do a direct fit rather than least-squares, taking the measured A\ value from Chapter 3: Model Synthesis 22 [1] and fitting the remaining coefficient A3 'by eye'. It was found that the most important characteristic of the data was the slope at zero, dC^/da \a-o, and the best results were obtained when this parameter was used to fit the data. Of course, other criteria, such as the location of the maximum lateral force coefficient, could be used, with nearly as good results. The polynomials used are observed in Figure 3.1.1 to underpredict the data by as much as 30%. This is a consequence of forcing the first coefficient to be as given. The turbulence levels measured in [l] were v'/V — 0%, 6.5%, and 10.5%, the low, medium, and high levels. The data are reproduced in Fig. 3.1.1 and compared with the polynomials fitted, and the polynomial fit coefficients are given below: Ak k Low Medium High 1 4.87 3.95 3.15 3 4.21 x 102 51.4 47.2 5 1.70 x 104 0.0 0.0 7 1.94 x 105 0.0 0.0 We have used a degree 7 polynomial to fit the low turbulence data in order to fit the characteristic double curvature of the data. The higher turbulence data does not have this characteristic, and qualitatively a cubic polynomial is sufficient to fit the data. Quantitatively, the polynomial fits are quite poor, but the simplicity gained by keeping only the degree three nonlinearity is worth the accuracy lost. Chapter 3: Model Synthesis 3.2 Experimental Determination of a, B, and D. 23 We will use the data reported in [2,16] to fix, for u0 = 1, the values of the remaining free parameters. Bearman and Obasaju carried out forced-vibration ex-periments with a square-section cylinder in cross flow, and measured the effect on the fluctuating lift on the cylinder. Obasaju [16] reported fitting the parameters in to his data. He reports CL0 = 1.4, a = 0.13, and B/CL„ = 0.179, for an amplitude ratio of 0.10. We compare this with the form from our model equations, with Y = Fsin(wO: Now, to « 1 in [16], and to make our form more compatible, we put E2LOQ = Y2(B2 + D2). Then we have DYcos{t) - BYsm{t) = £u>2,sin(* + 0), where 6 is defined appropriately. At resonance, (3.2.1) has the solution CL = C/>sin(f — 90°). If s'm(t) is in phase with cylinder velocity, then the angle <f> by which the lift CL leads the displacement is if) + 90° = 0°. If sin(t) is in phase with the cylinder displacement, then we have <j> = —90°. The measured <f>, however, is more nearly — 70°, than either of these. Noting that Y = 0.1 in the forced-vibration experiments, (3.2.1) CL - OLLO0CL + — C f + wlCL = Bui sin(wi) (3.2.2) Cv - a{u0) I Cv <lCv = DuY cos(u)t) - BLJ2Y sin(w*). Chapter 3: Model Synthesis we have 24 (3.2.3) E = 2.5 (3.2.4) ib-0 = -70 c thus 0 = -20 c so, at u»o = 1, B(l) = -2.5cos(20°) = -2.35 D(l) = 2.5sin(20°) = 0.855. Note also that a(l) = 0.13. Remark It is possible to determine more than just one value from this data. However, all the data in [16] is from the resonance region, and I believe that it is necessary to gather data outside the resonance region, and in particular in the subharmonic and superharmonic resonance regions, before this practice becomes useful. These values give a good fit with the CL observed in the resonance region (as Obasaju's already did), and a slightly better fit for the phase angle data. C h a p t e r 4 Methods of Solution of the Model Equations / myself have since, by divers ways, as many lines as meet in a dial's centre, come nearer the truth. —E. R. Eddison 4.1 D i s c u s s i o n of A v a i l a b l e M e t h o d s There are several methods in our 'kitchen' for finding an approximate solution of the model equations, each with their advantages and disadvantages. We shall consider four different approaches here: the method of Van Der Pol, the method of multiple scales, a bifurcation solution, and a direct numerical approach. This last method is the simplest in concept as well as the simplest in execution, but we shall see that in many ways it is the least satisfactory. All of the other methods reduce ultimately to numerical computation of one sort or another, but as is usual a computer is no substitute for thought. It is useful to note at this point that we use 25 Chapter 4: Methods of Solution 26 the symbolic manipulation language REDUCE [ll] for many of the computations that occur. REDUCE makes the manipulation of polynomials and asymptotic series easy, and in this context represents a proper use of a computer. The first method we consider is a natural one, the method of Van Der Pol [14,27,10]. We expect to see oscillation at or near the natural frequency, so we look for a solution of the form Y = Fcos(ta) (4.1.1) cv - cvcos(nt + v>) On substitution into the model equations, we get two inconsistent equations, in that the coefficients of the terms cos(3f2i), sin(3fl2), and higher frequencies, are not equal on both sides of the equations. However, we can insist that the coefficients of cos(Oj) and sin(fM) are equal, and this gives us four equations for the four unknowns Y, Cv, ip, and JI. Due to the polynomial character of our model equations, we will get four coupled polynomial algebraic equations. Theoretically, this is a step forward. Surprisingly, in spite of the dubiousness of ignoring the effect of the higher-frequency terms, this method is quite accurate (when we can solve the resulting polynomial equations). There are three main theoretical difficulties, however: No error estimate is available, so we do not know how accurate our solution is; there is no obvious way of computing the stability of the computed solution; and there is no provision for the sometimes-important higher-frequency terms. All of these combine to make Chapter 4: Methods of Solution 27 the method of Van Der Pol useful only as a first approximation. There is a further practical difficulty, more important if a more complicated form than (4.1.1) is taken, and that is the difficulty of solving systems of polynomial equations. There are many efficient methods for solving such systems: for example, the homotopy methods, which develop a system of differential equations with complex initial conditions whose limiting solutions are the roots of the original polynomial system, and use a numerical ODE solver to find these roots. It is amusing to note that this is the precise reverse of the classical technique for solving differential equations! In this case, this could still be justified by the fact that the resulting ODE's would be nonstiff, and much easier to solve numerically than the original system. We consider next a direct numerical solution of the model equations. There are many efficient methods for the solution of such initial value problems, and many existing packages which we can take advantage of. There are three problems here: expense; the fact that a numerical solution obscures the effect of the various parameters, and gives relatively little insight into the solution; and the fact that we must vary our initial conditions to obtain all the stable solutions, while the unstable solutions remain inherently undetectable. First, we consider the cost of solving the system. We add the following (variable) initial conditions to the model equations, variable because Chapter 4: Methods of Solution 28 we do not know precisely what the physical initial conditions are: Y(0) = Fi C„(0) = F 2 (4.1.2) y ( o ) = F 3 Cv{0) = F4 where the F{ are unspecified at present. Now, we need at least 10 values of the solution in each cycle, and we know from the experience of the Quasi-Steady model that the time taken to reach the limiting amplitude is 0(1 /n) as n —> 0. For n ~ 10 - 3 this means about 104 values need to be calculated; now, for a reasonable response curve we need ~ 100 values of the limiting amplitude; this is already ~ 106 operations, and this is for a single set of initial conditions. We must also vary the other parameters of the model equations. If we have the computing resources available (and they have nothing better to be used for), then this approach is reasonable. We can improve the efficiency a great deal if we risk omitting any disconnected solutions by using the method of continuation. That is, we use the limiting amplitude of the previous wind speed solution as an initial condition for the current wind speed. This is a closer model of what actually happens in a wind tunnel (the wind speed is increased or decreased gradually, and the oscillations are allowed to reach a steady amplitude from there). This avoids the great deal of time involved in reaching the limit cycle. However, we can do much better, at least for the case of small n, by using an asymptotic approach. As n increases, the cost of the direct numerical approach Chapter 4: Methods of Solution 29 decreases, while the asymptotic solution becomes less accurate. In this sense, the two methods complement each other, and this suggests that the numerical method is more appropriate for the case of oscillation in water, while the asymptotic approach is more appropriate for the case of oscillation in air. Of course, we would like the asymptotic approach to be useful for water as well. We consider two essentially different asymptotic approaches: the method of multiple scales [3,13,15,25], and a bifurcation approach [6,12,21,22]. The method of multiple scales uses the physical parameters present in the problem, n and a(uio), and produces a solution that is asymptotic to the exact solution as n —> 0 and a —> 0. As a device to aid in the solution of the resulting equations, we will assume that a oc Jn as n —> 0. This is reasonable, as the physical values of the parameters that we use are approximately of these orders, and in fact is crucial to the ease of solution; assuming that the two parameters are of the same order leads to a much more difficult set of algebraic equations. The idea for using this order of expansion came from an analysis of the solution of the model equations by the method of Van Der Pol near the resonance region, where the Van Der Pol solution was not precisely as expected. We note that the resulting equations are still quite complicated, and although the solution to first order is possible by hand with some degree of certainty, the next term is harder, and the use of the symbolic manipulation language REDUCE Chapter 4: Methods of Solution 30 is justified. The third terms, obtained as a check on the consistency of the solution and as an error estimate, would not have been obtainable by hand without heroic effort. For a solution, we get an asymptotic expansion in powers of n = y/n, and we hope that the physical value of n is small enough to give reasonable answers from the asymptotic solution, with only a few terms needed. We will find three time scales useful in our solution: T, characteristic of the time for one oscillation, TX = p,T ~ aT, the time scale on which the vortex excitation grows, and r2 = \i2T ~ nT, the time scale of the amplitude growth as in the quasi-steady theory. We should note at this point the different meanings of the 0(n) symbol to the mathematician and the engineer: to a mathematician, the phrase X = 0(n) as n —» 0 means precisely that the quantity X satisfies lim — = K < oo n—o n where K is any constant. To an engineer, the phrase X = 0(n) when n = 10 - 3 simply means that X is about 10 - 3. It is one of the more useful features of asymp-totic series that the constants K that come up are often of moderate size, so that the two meanings of 0(n) then approximately coincide; in fact, we often find that the constants are such that our asymptotic series give results far better than we have a right to expect. Here the method of multiple scales will give a solution of Chapter 4: Methods of Solution 31 the form Y Y0 + /xFj + p2Y2 + • • • (4.1.3) C, V c0 + nd + n2c2 + ••• and we shall find that we get good accuracy with only two terms for Y and one term for Cv. Further, the stability of the solutions is immediately available, as well as an asymptotic error estimate, although, as noted above, this is not the same thing as a practical error estimate, unless we are lucky. Thus, we still need some sort of assurance that our constants are not too large, and an estimate of the error made by taking so few terms. Thus we consider another asymptotic method, that used for bifurcation theory. As in the Hopf Bifurcation Theory, we introduce the new parameter e = u 0 —w,-, where CJ, is an easily-found value of the non-dimensional wind speed at which some pair of eigenvalues of the system linearized about 0 crosses the imaginary axis. As this parameter actually goes to zero physically, we know that this parameter will be small enough (at least in some region of the response curve) to provide an arbitrarily accurate solution. Some formulae for these calculations were worked out for the Hartlen-Currie model by Poore and Al-Rawi [21,22], and an adaptation of their work provides us with a solution which is very accurate near these Hopf Bifurcation Points and near the zero solution. This last restriction limits the utility of the approach, as all of the solutions found by this method are unstable, but these Chapter 4: Methods of Solution 32 are the only completely accurate solutions we have any information about, so they are useful in checking the other methods. It is also interesting and informative to investigate how these periodic solutions bifurcating from the zero solution affect the 'nearby-in-F' solutions predicted by, for example, the method of Van Der Pol. We find in conclusion that all four methods have their uses, and complement each other somewhat. The method of multiple scales is the method of choice for small n, but it needs checking; near zero by the bifurcation solution, and away from zero by the method of Van Der Pol. The numerical method is most useful for larger n, although we hope that the method of multiple scales will be useful even for quite large n, due to our experience with the surprising power of asymptotic methods. Chapter 5 Solution of the Model Equations by the Method of Van Der Pol And now,—thinking on't in cold blood— go, 'tis a thing not believable! —E. R. Eddison 5.1 Setting up the Equations We look for a solution of the model equations (2.1.1)—(2.1.2) of the form Y = F cos (fir) Cv = Cvcos(Vlt + ip). On putting these into the model equations, and ignoring the higher frequency terms, we have (1 - fi2)F cos(nt) = nU2{-f{Y) sin(m) + C„cos(n* + ^)) [ul - U2)CV cos(ftt + xff) = -a(u0)g(Cv) sin(fit + 0) - DflY sin(m) - BVl2Y cos(0*) 33 Chapter 5: Van Der Pol Solution where 34 f(Y) = P I { Q Y ) - P 3 ( f iY) 3 + P 5 ( n y ) 5 - p 7(nr)' n2c 2 g[cv) = n c v \ i - - T i and 3X 3 P3 = Pb Pi = 4U3 5^5 8Z75 35^7 64E/7 so, equating coefficients of sin(fl<), cos(Oj), we have (5.1.1) (1 - n 2 )F = nU2Cvcos(^) (5.1.2) 0 - nU2{f{Y) + Cvsm{rp)) (5.1.3) {ul - U2)CV = DUYsin(V0 - -Bfi 2F cos(^) (5.1.4) 0 = a{u0)g[Cv) + DnYcos(rp) + £ f l 2 Fsin (0) . This gives us four equations in the four unknowns fi, ip, Cv, and Y. We can eliminate tp from the (5.1.1) and (5.1.2) by using (5.1.3) and (5.1.4) as linear equa-tions in sin(V') and cos(^), and then squaring and adding appropriately (5.1.3) and (5.1.4) we get three polynomial equations in the unknowns fi, Cv, and Y. With Chapter 5. Van Der Pol Solution 35 E2 = n2D2 + U4B2, we have then (5.1.5) E2Y2 = (w2 - n2)Cv2 + a2g2{Cv) (5.1.6) f(Y)E2Y = -n2Bag(Cv)Cv + nD{uj2 - f ] 2 ) C v 2 (5.1.7) (1 - U2)E2Y2 = nU2 (-n2B{w2 - f2 2 )C u 2 - nDag(Cv)Cv^j Remark This is an approximate solution of the differential equations (2.1.1)— (2.1.2) in the classical sense; that is, we have "reduced" the problem of finding the solution of a system of differential equations to that of finding a solution of a system of algebraic equations. As stated previously, this is in fact a difficult numerical problem, in general, especially when we have no initial guesses for the roots of the polynomial system. For this system, however, we do not need sophisticated general polynomial system solver routines, as with a simple further approximation we can reduce the system (5.1.5)—(5.1.7) to a single polynomial in a single variable. If we had started with a more complicated form for the solution of the model equations, however, this ad hoc approach would not work, and we would need a good polynomial system solver. 5.2 Solution of the Polynomial Equations If we ignore solutions that have Y small, then we are led by (5.1.7) to the conclusion that f l 2 = 1 + 0(n). This simplifies the solution considerably. We have Chapter 5: Van Der Pol Solution 36 in this case (5.2.1) E2Y2 = (cu2 - l ) 2 C \ , 2 + a2g2(Cv) (5.2.2) E2Yf[Y) = Cv2D(u2 - 1) - aBCvg{Cv) and further, (5.2.3) O 2 = 1 + (B{u2 - 1) + aD(l - -£4) E2Y V CY^ — 2 We may substitute (5.2.1) into (5.2.2) to get a single polynomial equation in Cv , which is solvable by standard numerical methods. Remark Even single polynomial equations are sometimes difficult numerically, if there are roots that are close together. Here we do not have this problem, at least — 2 most of the time. This polynomial is degree 11 in Cv , and the coefficients were obtained by REDUCE for the FORTRAN program used to find the roots. The library routine RPOLYl was used, as it is efficient and reliable. Remark Now that we have provided an answer to the question of what the amplitudes are of the solution to the model equations, we would like also to answer the following questions: 1. How accurate is the solution? 2. Where is the solution stable, and where is it unstable? Chapter 5: Van Der Pol Solution 37 3. Are there regions where the higher frequencies become important? The first question is really unanswerable by this method. In ignoring the higher frequency terms, we seem to have made an error of 0(a) or O(n), but the details are not clear. The second question can be answered, but it is not simple. In [27], Wood carries out a stability analysis for a similar series of models of vortex-induced vibration. He does not, however, allow for a sufficiently general variation. Thus when he claims a root is unstable, his results are correct, but when he claims a root is stable, his results are unconvincing. We will find that the stability analysis is much easier, in fact automatic, when the method of multiple scales is used instead. The third question can be addressed by using a more complicated form for the solution, instead of Y cos(fi£) and Cvcos(Ut + tp). If we include higher-frequency terms (although it is difficult a priori to decide which frequencies to include), we should get more accuracy, and be able to tell when the higher-frequency terms are important. However, the polynomial systems that arise become unwieldy rather quickly, with each new term added, and as the method of solution in this case was rather ad hoc, this is not practical. 5.3 Results of the M e t h o d of V a n Der Po l The following figures, Figure 5.3.1 and Figure 5.3.2, show the results of the Chapter 5: Van Der Pol Solution 38 method of Van Der Pol compared with data taken from [l]. We compare with the low turbulence data only, as illustration. We see that the agreement is quite good, except in the medium damping case near the upper range of values. We see some of the features of the quasi-steady model present in the solutions of this model, notably in the medium damping case, where we see three branches of the solution. There is a qualitative difference from the quasi-steady solution, however, in that a new branch of the solution is present, continuing the lower branch of the solution past UQ « 5. When we compare this solution with that from the method of multiple scales, we see that this new branch is unstable. Comparison of this solution with experimental data is problematical in this case. The lower branch of the curve agrees quite well with the data, but one would have expected the experiments to show the upper curve as well, as for UQ < 5 they appear to be within the range of measurement. However, past LOQ « 5 for the medium turbulence case, this model predicts that the upper branch would be outside the allowable deflections of the physical model. Since the upper branch can be detected only by decreasing the wind speed from a speed at which the upper branch is established, it may have been that the upper branch was in fact not detectable with the physical model. This could be verified by repeating the experiments, and giving the model a "bump" in the indicated wind speed range, to see if the upper branch could be detected. However, the lack of an upward curve in the data near the end of the predicted range of the lower stable Chapter 5: Van Der Pol Solution 39 branch indicates to the contrary that the upper branch is not located correctly by the model equations. Another curious feature is the "V"-shaped curve at the beginning of the high-damping case. Again, the later solution by the method of multiple scales shows that the left branch of the "V" is in fact unstable, leaving a more usual-looking curve. The solution in the resonance region is not clear from the graph, but other investigations not reported here have shown that the solution in the resonance region consists, for the high-damping case, of a "double humped response". The solution in this region rises from zero before exact resonance to a peak, and then returns to zero precisely at resonance. This is followed by a second rise to a peak and then back again to zero. The method of multiple scales predicts similar solutions, but as we shall see in Chapter 7, different in detail. It is worth noting that the unexpected return to zero at exact resonance is an artifact of the method used to solve the polynomial equations, and that a more exact solution does not have this feature. It is consideration of this that led to the proper asymptotic form of the solution used in the method of multiple scales. The low damping solution appears to be overpredicted just after the resonance region, perhaps by as much as 40%. Also, the kink near uo « 3 is not reflected in the solution. If in fact this is a subharmonic resonance, this is to be expected. The method of Van Der Pol is, in this simple form, incapable of describing the effects of Chapter 5: Van Der Pol Solution 40 the higher frequencies. One good feature of the solution of the model equations for the low damping case is that the nonzero solution begins near wo ~ 1, and not at the value predicted by the quasi-steady theory. This is a major qualitative feature of interest. The quasi-steady model was incapable of reflecting this feature, observed experimentally. Chapter 5: Van Der Pol Solution 41 Figure 5.3.1 Van Der Pol Solution in the Low Turbulence Case. Chapter 5: Van Der Pol Solution 42 2-i 1.8 H 1.6 H 1.4 H 1.2 H 0.8H 0.6 H 0.4 H 0.2 H 0 A A 'A •0 © $ o o V v° o o' o o 2 3 T 4 5 a = 0 . 1 J x u 0 ' D = 0 .85 V«0 6 = - 2 J 5 / « 0 2 A c 1 .87 A A Legend • Von DOT- Pol Solution o tow Dumping » Madfcjm Domping • High Damping 6 [LJ HI U 9 Figure 5.3.2 Excitation by the VDP solution in the Low Turbulence Case. Chapter 6 Hopf Bifurcations of the Model Equations But first I would have you, as a politic prince who will not lay your foundations in the dirt but on archaean crust, refer the whole estate to your highness' delib-erate overviewing again. —E. R. Eddison 6.1 Introduction In view of the fact that the model synthesis is semi-empirical, we must be somewhat more cautious in applying traditional methods of approximate solution. For example, we have no a priori assurance that the solutions to the model equations are sensible periodic solutions, or indeed exist at all. Also, we have seen that if we wish to apply the Method of Van Der Pol to solve the equations, it is helpful to have some idea of the form of the solution, and we will see that for the Method of Multiple Scales, it is helpful to try to estimate the effect of the size of the 'small' mass parameter n. This ideally would permit investigation of the model 43 Chapter 6: 44 for both the aerodynamic and the hydrodynamic cases. Thus we must try to find as much information about the exact solutions to the model equations as possible before putting any faith in the results of our approximate solutions. Of course, we cannot hope to solve these nonlinear equations exactly, but there are certain parameter values near which we can say a great deal about the solution, by the use of the mathematical tool, Hopf Bifurcation Theory. Hopf Bifurcation Theory provides much useful information about the exact solutions of certain kinds of nonlinear equations, and also provides a method of calculating an approximate solution, guaranteed to be accurate in some (possibly small) neighbourhood of the zero solution. This will give us information about the model equations that will be valid for all values of the mass parameter n, and thus will include both the aerodynamic and the hydrodynamic cases. Of course, the theory has its limitations, which will be discussed after the basic ideas have been explained. An elementary, if somewhat terse, introduction to Hopf Bifurcation Theory can be found in [12]. 6.2 H o p f Bifurcation Theory This theory predicts the bifurcation of periodic solutions from steady-state so-lutions (in our case the zero solution) of nonlinear differential equations. Let the Chapter 6: 45 equation be written as x = A(OJ0)X + f(x,u>0) where x = (x,... ,xn)T, A(u0) is n x n, / is the strictly nonlinear part of the equations, and is a scalar parameter. The theory locates values of the parameter CJO, denoted w,, at which a periodic solution is initiated, and gives a method for finding the direction of bifurcation, the frequency of oscillation, and the amplitude and stability of this periodic solution, all in a neighbourhood of the critical value of u>o and the zero solution . The basic idea of the theory is to first find the critical values of u0, called Hopf Bifurcation Points (HBP's), and then use a local coordinate transformation to change the possibly strongly nonlinear equations to a set of weakly nonlinear equations, with a new parameter p which is proportional to u>o — LO{. These weakly nonlinear equations can then be solved in an asymptotic sense, and this asymptotic solution gives information about the exact solution in a neighbourhood of /i = 0. This analysis does not depend on the possibly small mass parameter n, but rather on an artificially introduced new parameter which is guaranteed to be small enough, at least in a neighbourhood of the Hopf Bifurcation Point. The first task is to locate these Hopf Bifurcation Points. This is easily done, as they are the values of UQ for which some pair of eigenvalues of A(uo) cross simply the imaginary axis. When the equation is linearized at this point, the resulting linear equations have a purely Chapter 6: 46 periodic solution. This is the basis of the theory, and of the asymptotic solution of the new weakly nonlinear equations. Thus if the eigenvalues of A(u>0) are Ct(wo) the HBP's are the roots of Re(a(w0)) = o subject to ImfoK)) + 0 3Re(fiM) 0 If all the other eigenvalues of A(OJO) have negative real parts, the HBP is also associated with the loss or gain of stability of the zero solution, as the parameter LOO is varied through the HBP. In our model, the bifurcation parameter is the dimensionless wind speed u0 (or equivalently U = UroJo). Before proceeding with the analysis, we note that Poore and Al-Rawi [21,22] have developed formulae for the direction, stability, and amplitude of the periodic solutions for general ODE systems. They applied their formulae to the Hartlen-Currie model of vortex-induced vibration, and a similar application to this model is desired. 6.3 Bifurcat ion Formulae [21,22] With some notational changes, the following theorems and formulae are taken Chapter 6: 47 from [21,22]: Let x = My (1 + = t e = fi6 = u>0 — wt (/x > 0) A £ = A[u>0) = i4(wt- + e) eBE = A£ - A 0 B ^ = d ^ - \ e = 0 = A'(u)l) M2Q(y,M,^) = /(My,wt- + e) This transforms the differential equation (5.1) to — = A°y + nG(y,n,6,i) where G = SB^y + -yA^y + (1 + M7)Q Notice that the equation for y is a weakly nonlinear equation, in that as Do —• wt, // —* 0. The theorems and formulae reproduced below are a consequence of the fact that this weakly nonlinear system of equations may be solved much more easily than the original system, and as the artificially introduced parameter fi does go to zero in a region of interest, we are guaranteed that the formulae given below will apply, at least in some possibly small region around the HBP. For details of this process, see [12]. The parameter 6(fi) = 6(0) + fi6'(0) H can be shown to have 6(0) = 0; thus Chapter 6: 48 p2S'(0) « w 0 - w,- and then the sign of 6'(0) gives the direction of bifurcation. The parameter 7 represents a detuning of the frequency of the oscillation, and it can be shown [12] that the amplitude of the bifurcating periodic solution is proportional tO y/jl. We know that at the Hopf Bifurcation Point, some pair of the eigenvalues of A(UJQ) are purely imaginary. Let r(e) ± ifo(e) be the continuous extension of these purely imaginary eigenvalues. We are now in a position to reproduce three theorems [21,22] which reduce the bifurcation problem to an explicit algebraic computation. T h e o r e m 1 [21] Let F(x,e) € Ck [D x { —eo,£o)} for some EQ > 0, k > 3, and D a domain in R 4 containing 0. We assume that A0 has a pair of complex conjugate purely imaginary eigenvalues ±t / o with fo > 0, and if A is any other eigenvalue of A0 then A ^ 0 and A ^ ±imf0 for any integer m. Let r(e) + ifo[z) denote the eigenvalue of AE which is a continuous extension of +ifo and let T — 2TTjfo. If r'(0) 7^  0, then for some sufficiently small pi > 0 there exist real valued functions 6(p) and ^(p) G C^k~2)\—p\,p,\\ and a T-periodic function y(s,p) such that 6(0) = 7(0) = 0 and x(t,p) = nyt 1 p) \1 + M 7 ( M ) / Chapter 6: 49 is a (1 + p^(p)) • T-periodic solution of ~ = A£x +F{x,e[p)) for e(p) = pS(p). If 6 = 6(p) and 7 = i{p) in the transformed equation ~- = A°y + pG{y,p,6,i) ds then y(s,p) is a T-periodic solution of this transformed equation. Theorem 2 [21] (stability result) If k > 4, r'(0)6'(0) > 0, and Re(Af) < 0 for the other eigenvalues, then the bifurcated periodic solution will be asymptotically orbitally stable. Theorem 3 [21] (algebraic expressions) If u and v are the left and right eigen-vectors of A0 corresponding to the eigenvalue +ifo, normalized so that u • v — 1, and B is any nonzero real two-dimensional vector, then r'{0) + if0'{0) = uB0v and 8r'(0)(5'(0)+i8(/0(0)^(0) + /o7'(0)) d3Fl _ d2Fl 0 ! d2Fr BBl -ui-—-—-—VjVkVp + 2ui-—-—VJ(A )KR dxjdxkdxp dxjdxk dxpdxq VpVq Chapter 6: 50 Poore and Al-Rawi remark that as e = nS = n26'(0) + 0(/J,4), the periodic orbit bifurcates to e > 0 when 6'(0) > 0 and to e < 0 when S'(0) < 0. They further note that the initial conditions on the periodic orbit may be approximated by / £ / ~ (v — v) ' „ (v + v) \ where B — (B\,B2) is any real nonzero vector, essentially representing the choice of initial conditions, and v is the same as in Theorem 3. Poore and Al-Rawi used this last observation as initial conditions for numerical solution of the equations in the neighbourhood of the Hopf Bifurcation Point — we will use it for an analytical approximation to the amplitude of the periodic orbit near the HBP. 6.4 Bifurcat ion of the Quasi-Steady M o d e l In this section we will illustrate the ideas of Hopf Bifurcation Theory by using the results of the previous sections to analyze the simpler quasi-steady model of galloping due to Parkinson [17]. The model equations are Y-+Y = where n, A\, A3, . . . and L70 are empirical constants. This is a two-dimensional Chapter 6: 51 system, and written in first-order form, with X\ = Y and x2 = Y, we have 0 1 X\ | 0 i2 -1 nAx{U-U0) . Z 2 . -T - n A z ~ Z | , [ y x 2 - T The eigenvalues of the linear part of the equation are easily calculated explicitly: nAi{U - U0) ±iJl- {nAiiU - U0))2 f = 2 and for |n^i([/ — U0)\ < 1 we see that Re(f) = n>(i(l/ — U0)/2, which is zero if and only if U = I/o, while a ^ = nA\\2 ^ 0. Thus the only Hopf Bifurcation Point of the Quasi-Steady Model is at the point U = UQ. This is in accord with the approximate analytical solution. There remains the calculation of the direction and amplitude of the bifurcated periodic orbit. By straightforward calculation using the formulae of Poore and Al-Rawi, we have and r l i ]T v=l75 73J so, choosing B = [l, 1], we get 8 r W ( 0 ) + « ' ( 8 V ( 0 ) ) = ^ Chapter 6: 52 which gives "/(O) = 0 and so we see that the periodic orbit bifurcates for U > Uo, and in fact is stable. By straightforward use of the formula for the initial conditions on the periodic orbit, we deduce that the amplitude of the stable bifurcated periodic orbit is which is precisely that obtained by the approximate solution in the small n case when As — A7 — 0 by the method of Krylov-Bogoliubov, used by Parkinson and Smith [20]. For a comparison of the two solutions, see Figure 6.4.1. This result is somewhat surprising, as it is independent of n (one expected some terms of order n, n 2 , etc cropping up). Note that this solution is valid even if ^ 5 , A7 ^ 0, but we are only guaranteed accuracy when U is near C/0. Also, no form of the solution was assumed a priori, and the oscillatory nature of the solution was derived directly from the differential equations, and we are guaranteed that the actual solution of the differential equations does in fact look like this, in a neighbourhood of UQ. This enables us to draw a local response diagram which we can compare in this simple case with the well-known approximate solution. When we examine Figure 6.4.1, we see that the two solutions given agree best near U = Uo, as predicted by the theory. The agreement remains quite good for a Chapter 6: 53 0.50-1 Figure 6.4.1 Comparison of the Bifurcation Solution to the solution by the K-B Method [20]. reasonable range of wind speed values, but eventually diverges, as the assumption that U « Uo is violated. Also, the global features of the approximate solution pre-sented in [20], notably the two branches of the solution, are not predicted by the bifurcation theory. It is interesting to note that if As = A7 — 0 these curves would coincide precisely, so we would have in that case obtained a globally valid solution by local considerations only. This must be regarded as a coincidence, and it is not expected to occur in the more complicated model we are interested in next. To summarize, the Hopf Bifurcation Theory gives us formulae that predict the loca-Chapter 6: 54 tion(s) in parameter space at which periodic solutions to the differential equations are initiated, and allows us to calculate the local behaviour of such solutions. This is of interest physically, as the wind speeds at which nonzero amplitude vibrations are initiated are important design parameters. It is also important for the theoretical investigation of models for such vibrations as unrealistic behaviour is detected at an early stage. 6.5 Limitations of the H o p f Bifurcation Theory The theory is essentially local: it cannot provide information about the solution of the equations away from the Hopf Bifurcation Points, or away from the steady state solution (the zero solution) that the periodic solutions bifurcate from. Thus isolated branches of periodic solutions are not predicted (as in the experimentally observed closed loops of Wawzonek), and secondary bifurcation from the periodic solution is not detectable with this simple analysis. It is the latter bifurcation that we are more interested in, as the zero solution of our model equations is always unstable, and hence any physically observed bifurcations are in fact bifurcations from a limit cycle solution, and not from the zero steady state. It is important to note that by zero solution we mean the solution Y = 0, Cv = 0, which is the only steady-state solution of the model equations. The fact that this solution is unstable follows from the fact that the damping in the second equation is negative, Chapter 6: 55 at least for small values of Cv. However, we will find that these solutions will be useful as error checks for the other methods of solution, and as a quick indicator of the behaviour of the solution. The interaction between the steady-state bifurcation analysed here and the secondary bifurcations that are observed are interesting of themselves, and worth further study. 6.6 M o d e l Eq u a t i o n s The model equations that we shall be analysing are reproduced here for conve-nience: * + . - ^ ( . 1 ( 1 ^ ) | - A ( ^ + ,.g) ,.. r(*)' + c.) Cv + u,20Cv = a(cu0) (dv - -rp^—ici] + DY + BY Naturally, the details of the location of the Hopf Bifurcation Points will depend on the exact nature of the functions a(u>0), B(ui0), D(u!0), and Cy ( ). The analysis itself, however, is not so sensitive. Once we get down to details, the models we will actually investigate are the Hartlen-Currie model, with a(u>o) = awo, and Bouclin's hydrodynamic model, with a(carj) = GCy , where a, G, Cy ( ) (and all the other parameters) are constants. Chapter 6: 56 6.7 Locat ion of the Hopf Bifurcation Points To locate the Hopf Bifurcation Points, we use only the linear part of the equa-tions. We change the notation slightly, putting x\ = Y, x2 = Y, £3 = Cv, and £4 = Cv, and writing the matrix as: (6.7.1) • 0 1 0 0" A — -1 t(u0 - W0) 0 0 0 0 1 . —B D+e{u0-W0)B -ul + enulB a. where e = nA\UT, n = and W0 — jj This matrix has the characteristic polynomial P(f) = a 0 + aif + a 2f 2 + azf + f4 where (6.7.2) a0 = ul ai = - (a(u0) + enDul + eul(u0 - W0)) a2 - 1 + ul + a(u0)e(u0 - W0) - Berjul «3 = - (a(wo) + e(w0 - Wo)) Notice that the effect of the additional BY coupling term is confined to the coeffi-cient of f 2 . Now, when are some pair of roots of P(<r) purely imaginary? One way to find Chapter 6: 57 out would be to use the analytic solution of a quartic equation to try to find smooth expressions for the roots of P(c), and then try to find the parameter values for which some of these roots had zero real parts. This is tedious, except in the limit as n —• 0, when reasonable expressions can be obtained for the roots of P(f). It is easily seen that and if n <C a then the Hopf Bifurcation Points are the zeros of OI(LOQ). Note also that for small n, Re(f3) = a/2 -+- 0(n) > 0, so any bifurcating periodic orbit is initially unstable . However, there is a simpler method that works for all values of n, and not just those which are small compared to a. When the roots of P(f) cross the imaginary axis, they do so in pairs. Thus the polynomial f 2 + / 2 , say, is a divisor of P(c) at this point. By long division, So at a Hopf Bifurcation Point, the remainder must be the zero polynomial. We thus get two equations in the two unknowns f2 and UQ, as follows: Ci(wo) = i + n- ffi(wo) + 0(n2) + n-o2 + 0(n2) Pit) = (C 2 + f2)Q($) + (ai - a 3/ 2)c + a 0 - (a 2 - / 2 ) / 2 (6.7.3) « i - a3f2 = 0 (6.7.4) ao - a 2 / 2 + f4 = 0 Chapter 6: 58 This system of equations applies for all n, and we can reduce it to a single equation quite easily. If a 3 ^ 0, then f2 = ai/a^, which is required to be > 0. Substituting in the second equation gives a single equation in OJQ : P B (C J 0 ) = a\a0 - aia2a3 + a\ = 0 (6.7.5) Any root of this equation is a candidate for a Hopf Bifurcation Point. If, however, 03 = 0, we are led to the possibility of a double bifurcation , P(c) = U 2 + fi )(C2 + /!)• I f °3 = °. t h e system (6.7.3)—(6.7.4) becomes (6.7.6) a x = 0 (6.7.7) a 0 - a 2 / 2 + f4 = 0 If equation (6.7.7) has positive roots for some selection of the parameters, then this is a double bifurcation point and must be handled specially. The bifurcation theory for this case has been worked out [21,22], but we shall see that the actual occurrence of this in our model is too rare to warrant special consideration, as any special features can be derived by taking limits. 6.8 Coefficients of the B i f u r c a t i o n P o l y n o m i a l For Bouclin's model, we take B(w0) = 0, a(w0) = GCY constant, and D(u0) = Chapter 6: 59 H, also constant. If fj = ^ and g = GCYu, we find by REDUCE that PB{UQ) = C 5CJQ + C4UQ + C 3CJQ + C 2WQ + CiOJo + c0 where c 0 = W0g{l + g2 - eW0g) C l = -g{l + g2 - 2eW0g) c2 = rjg- 2W0g + e (fjWog2 + Wo -g2{l + W2)) + e2gW2(WQ - rj) c 3 - 2g + e (2W0g2 - 3(1 + g2)) + e2W0g [2f, - 3W0) c4 = (W0 - rj)g + e{fj2 - fjWo - g2) + t2{-fjg + 3W0g) cs = -o + f-fj - e2g Notice that the only dependence on j3 is through W 0 = U0/Ur = 20jnA\\Jr, but that e depends on n also, so the roots of P B ( ^ O ) depend on /3 and n independently, unless n is so small that terms of 0(e) may be neglected. Thus a graph of Z7t- versus P/n is insufficient, except in the case of small n. For the original Hartlen-Currie model, we take B{UJQ) — 0 and D(u>o) = H as before, but a(u>o) = awo where a is a constant. This changes the character of P B (u; 0 ) markedly. We find again by REDUCE that P B ( ^O ) = C&UQ H h ciuo + 0 so in this case LOQ = 0 is always a root of the bifurcation polynomial. However, by Chapter 6: 60 inspection we see that for OJQ = 0, / 0 = 0 also, so this is not a Hopf bifurcation point. The coefficients ct are given by: c2 = -a + e{fjWo ~ CL2W2) c3 = a(f)+ W0{a2 - 2)) + e{2W0a2 - f,) + e2W2a{W0 - fj) c4 = a(2 - a2) + 6 (r7(/? + W0a2 - W0) - a 2 ( l + W2)) + e2W0a[2fj - 3W0) c5 = a{W0 -fj) + e (2W0a2 + - a2)) + e2[-rja + 31¥ 0a) c6 = —a(l + ea + e2) R e m a r k Both polynomials have roots which approach W0 as W0 —»• oo, which is realistic. The asymptotic form for these roots is the same for each polynomial: As e —> l - , one root of Bouclin's model goes to oo as the leading coefficient goes to 0. This may be unrealistic, and the Hartlen-Currie model does not have this problem. As e —> 0, both polynomials approach the corresponding initiation polynomials derived from the approximate analytical solutions obtained by the Methods of Van 0 Wna Wi = Wo-rj + 0[ — ) as W0 -> oo Chapter 6: 61 Der Pol and Multiple Scales. This is to be contrasted with the quasi-steady case, where the bifurcation polynomial was exactly the initiation polynomial, and the dependence on n dropped out completely. R e m a r k Note that for each functional dependence of B(u>o), D(u0), and a ( w 0 ) that the polynomial P B ( w O ) has a different form. Strictly speaking, it is a polyno-mial only for certain forms. However, we are concerned only with at most rational forms for the parameters, so we will always have a polynomial in WQ to deal with. 6.9 R e s u l t s of B i f u r c a t i o n F o r mulae Using the formulae from Poore and Al-Rawi's Theorem 3, we have the following results, tabulated here for convenience. If t is an eigenvalue of A, then the left and right eigenvectors associated with <; are « = [ - ( f ( f - o ) + w g ( l - « 7 6 ) + 6)/c f(?-a)+w 0 ( l -o7&) t - a 1] & C 2 + l - e ( u ; o - W „ ) ? f ( f ' + i - e ( M „ - | y u ) t ) 1 R except for the normalization, u • v = 1. To satisfy this criterion, we divide each of u and v by ±> / |u • v\. Now, with B° = J^-, and B = [1,1], we have r'(wi) + »'/'(<".•) = u B ° v Chapter 6: 62 and 8r'{u,i)6'{u,i) + i • 8 [/'(w '^K) + /K)7(^ )] / dzF2 2_ d3F4 2_ where d3F2 _ -6A3n dx3 ~ U d3F4 _ -8a{u0) These formulae allow us to calculate, for any given set of parameters, the location, direction, stability, and amplitude of any bifurcating periodic solutions of the dif-ferential equations. A F O R T R A N program has been written to do this for a range of W0, given the other parameters. This allows us to plot the location of the Hopf bifurcation points versus the critical wind speed W0. From experimental evidence, we expect that the bifurcation points will approach 1 and W0 as W0 —> oo, if the model is realistic. From Figures 6.9.1—6.9.2, we see that this is not in fact the case. Figure 6.9.1 shows the location of the HBP's obtained using the functional form a(uo) — O J W O , for a constant value of n = 4.7 x 10~4 and for varying /?, so V^ o = 20l(nA\Ur) varies also. There is an HBP that approaches Wo as Wo —> oo, but the HBP's near 1 disappear for W0 > 3.6. As W0 goes to 0, the HBP's coalesce and go to l , except for Wo < 0.5, when we have two new HBP's appearing. These appear to be unrealistic, but they occur for values of /3 too small to compare with experiment, at least in the aerodynamic case. Chapter 6: 63 Figure 6.9.2 shows the location of the HBP's obtained with a larger value of n, n = 7.32 x 10~2 but with the same functional form, compared with the location of the HBP's obtained with a(u/o) GCY , constant. This figure shows the difference in predictions for the two types of models, and by comparison with 6.9.1 shows the effect of a small change in the value of n. We see that the predictions of the two models are quite different, and quite sensitive to the value of n. In Figure 6.9.2, the graph of the location of the HBP's for a(u>o) = au>o has at least one HBP for all values of the critical wind speed W0, while the model with a = constant has a range of W o for which there are no HBP's. The asymptotic behaviour of one branch of the solution is apparently the same as the asymptotic behaviour of one branch of the solution for the other model. This branch apparently has u>, ~ W0 as W0 —» oo, which agrees in the limit with the quasi-steady model. Thus both models seem to agree in the quasi-steady limit. The location of the HBP's does depend strongly on n, however, as we see com-paring Figures 6.9.1 and 6.9.2. There is still the branch approaching W0 as W0 —> oo in both cases, but the locations of the HBP's for small Wo are quantitatively and qualitatively different. In the larger n case we see that the HBP which was near 1 in the smaller n case has moved to a value above 2. This suggests that graphs of U{ versus /?/n as presented in [19] may be insufficient to capture the full functional dependence of Z7, on 0 and n. Chapter 6: 64 We present in Figs 6.9.3—6.9.5 the bifurcation solutions compared with the low turbulence data of [l]. The data are compared with the solutions obtained with the functional form a(uo) = au)Q. Again the agreement for the medium and high damping seems reasonable, except for the resonance region. The medium damping case has at least the correct qualitative features predicted in the resonance region, but the amplitude is vastly overpredicted. The fact that the predicted amplitudes in the resonance region cross is of no physical significance, as the curves are valid only in a neighborhood of the zero solution. Thus very little information about the resonance region can be deduced from the Hopf Bifurcation analysis. The bifurcation point for the onset of galloping is much better, and in fact gives good quantitative results. Because of the local character of the bifurcation solution, only a few points were generated by the computer program. In the medium damping case, it was of interest to extend the curve to compare the global behaviour. This extension shows that in the medium damping case the global agreement with the data of [1] is quite good, up until LJO « 3.0. Note that the bifurcation point is at CJO = 2.00, so the supposedly small parameter uo~Wi is about 1.0 at this point. Thus we see that even though the assumption that the parameter is small is violated, we can still get good results. This is similar to the coincidence noted in the bifurcation solution of the Quasi-Steady model equation. The resonance solution in the high damping case is not even correct qualitatively, Chapter 6: 65 with the bifurcating amplitudes apparently going in the wrong direction. However, at least they indicate that something of interest is occurring in that region. For the low damping case, even this much is not true. If we compare this solution to the complete resonance region solution by the method of multiple scales, or the solution in the resonance region by the method of Van Der Pol, we see that this bifurcation is the beginning of an unstable solution that occurs before the actual resonance region, and that the occurrence of a stable nonzero solution for Y must in fact be a secondary bifurcation, bifurcating from the periodic solution near Cv = Cy ( ) cos(T + 0), Y small. These observations support the assertion that the bifurcation method is useful as a preliminary and supplementary solution but does not give the complete solution. Considering that the onset of the galloping amplitudes is also in fact a secondary bifurcation, it is remarkable that the bifurcation theory gives anything useful at all in this situation. Yet we see apparently good agreement for the values presented. Chapter 6: 66 5 - i n = 4.7x10 4 a = 0 . 1 3X«Q 4 . 5 - D = 2.50 B = 0.00 4 - A = 4.87 1 *" K K 3 . 5 -K K K K K K K K K 3 -K a A A A A A ZD \ 2 . 5 -A A A A A A A A Z> A A A A 2 -A A A A A A 1.5-A 'A 1-'A 0 . 5 -A A A A A U r i i i t i i i i i i 0 0.5 1 1.5 2 2.5 3 3.5 4 4 .5 5 VV = u / u 0 Cr r Figure 6.9.1 Location of HBP's compared with the Quasi-Steady Crit-ical Parameter Uo/Ur = VTQ. Chapter 6: 67 a = 0.13 4 . 5 - D = 2.50 B = 0.00 A f = 4.87 n = 7.32xl0~ 2 4 -3.5-3 - o o ZD \ 2 5 -Z) 2-o o P ° ° o 0 o o o o o o o o o o o 8 0 0 0 0 o o V- o © o 1.5-1-L e g e n d o a = O C C J Q 0.5-v a = a o 1 1 1 1 i i i i i i 0 0.5 1 1.5 2 2.5 6 3 5 4 4.5 5 V = U r / U Cr r Figure 6.9.2 Comparison of the Two Functional Forms for the Wake-Oscillator Damping Chapter 6: 68 O.IO-. 0.09-0.08 0.07-0.06->- 0.05-0.04 0.03-0.02 0.01-0.00 n = 4.7x10 a = 0 . 1 3 X U Q 1 D = 0.855/w0 B = -2.35/W0: C Y = 1.40 T0 A1 = 4.87 = 4.21x102 Legend Hopf Bifurcation o Low Damping Data [ 1 ] 1 1 r 1 1 1 1 1 1 1 0.4 0.5 0.6 0.7 0.8 0.9 1 1.1 1.2 1.3 1.4 0 Figure 6.9.3 Bifurcation Solution in the Low Turbulence, Low Damp-ing case. Chapter 6: 69 Figure 6.9.4 Bifurcation Solution in the Low Turbulence, Medium Damping case. Chapter 6: 70 0.50 -i n = 4.7x10 - 4 0.45 0.40 H 0.35 H 0.30 H a = 0.13xwQ D = 0 . 8 5 5 / « 0 B - -2.35/W 0 : C Y = 1.40 T 0 A 1 = 4.87 A 3 = 4.21x102 Legend • Hopf Bifurcation A High Damping >- 0.25H 0.20 H 0.15 H 0.10 H 0.05 H 0.00 0.5 1.5 A A A A I 2.5 3 A A A —I 3.5 4 4.5 5 Figure 6.9.5 Bifurcation Solution in the Low Turbulence, High Damp-ing case. C h a p t e r 7 Solution of the Model Equations by the Method of Multiple Scales 'Tis a first point of wisdom, to affirm nought upon hearsay. —E. R. Eddison 7.1 O v e r v i e w a n d C h o i c e of T i m e Scales The choice of time scales is the key to a successful solution of the model equa-tions. After a certain amount of preliminary investigation, we are led to choose the following: T = nt Tk = pkT k = 1,2,3,4 where $7 = 1 + po\ + p2o2 + p3&3 H — and the o\ remain to be chosen. We wish to associate p with a(uo) (the parameter characteristic of the damping of the second oscillator), while p? is to be associated with n, the mass parameter of the first oscillator. This approach is reasonable 71 Chapter 7: Multiple Scales Solution 72 for the values of the parameters that we are interested in, and mathematically convenient in that it decouples the resulting equations. Associating n with n leads to coupled equations, while associating n3 with n increases the amount of work necessary without substantially improving the results (although in our case, since we have a(iu0) = O ( l 0 _ 1 ) and n — O(10~ 3) we would expect better results from letting n fa a(u0)3). To be more precise, we let p = Jn and define g = CL(UJO)/(J,. This presumes that we will find the numerical value of g to be not too far from 1, and in practice this is the case. Remark We will find that only the first three scales, T, T-J , and r2, are necessary for consistent results. In [13], it is noted that for the calculation of terms to 0(p2) for a general system of this type, we should need the additional time scales /x3T and p4T, but due to the fact that we will be looking for steady state solutions only, we will see that the first three time scales will suffice. The higher-order time scales are included for completeness. Our equations become (7.1.1) Y + Y = f*2 (jiY - r3Y3 + r5Y5 - r7Y7 + sCv^ (7.1.2) Cv + u2Cv = ngCv - PIC3 + DY + BY where ng = a(uo), m = 4a(ojo)/{3CYou2), p2r\ — nAi(U — t/0), fx2s = nil2, and li2r{ = nU2AilUi for i = 3,5,7. Chapter 7: Multiple Scales Solution 73 Remark Note that most authors solving systems of this type assume that B and D are small; that is, O(fi). When the numerical values are inserted, they are usually not small at all. This inconsistency does no harm to the solutions as they are after all coefficients of linear terms, which never present any difficulties. Here the inconsistency is avoided, by explicitly allowing B and D to be O(l), as they are experimentally [2, 16]. The derivative operators are then, to 0(fj,4), dt dt2 a ( a a \ 2( a a a \ a a a a a \ + f\°*dY+°*dT1+°>dT2+aiaTs + dT4) + a2 ( a2 a2 ar2 dTdTl dT2 + + 2-dTdT! ' dT2 ' ~dTdT2 a2 (2a3 + 2o- l t r 2 )— + 2{o\ + 2*2) d J . d a2 a2 a2 a2 + 2 _ „ +2ffx— +4oinmn +2-dTdr3 dr2 dTdr2 dT\dT2 + (7.1.3) (7.1.4) and finally, our solution will take the form (7.1.5) Y = Y b ( r , r , , T 2 , r 3 , T 4 ) + ^ i ( I > l 5 r 2 , r3) +/x 2y 2(T, r l 5 r2) + • (7.1.6) Cv = C0(T, 7 - i , r 2 , r 3 , r 4 ) + / i C i ( r , r i , r 2 , r 3 ) + ••• Chapter 7: Multiple Scales Solution 74 Before proceeding with the solution of the model equations, we give a brief overview of the organisation of the solution. The equations (7.1.1) and (7.1.2) are replaced by a sequence of simpler equations at each order. Equation (7.1.1) will give rise to the First O(l) equation, the First O(n) equation, the First 0(ju2) equation, and all the higher orders. Equation (7.1.2) will give rise to the Second O(l) equation, the Second O(p) equation, and so on. We will solve the O(l) equations first, and then proceed sequentially to the higher orders. Of any given order, the First equation will be solved before the Second, as we will find that the second equation depends on the solution of the first, but not vice versa, so they are effectively uncoupled. Each equation after the 0(1) equations will give rise to an anti-secularity equation for determining the dependence of the previous terms on the higher-order time scales. When the 0(l) equations are solved, we will find the solution divided into two cases by the Second O(l) equation and the requirement that the solution be bounded. We will see that the solution to the Second O(l) equation will be different depending on whether the wind speed is in the resonance region or not. This affects all subsequent equations. When the O(fi) equations are solved in the nonresonance case, the Second 0{fi) equation will give rise to two new subcases, the subharmonic resonance case when a»o ^ 3, and the superharmonic resonance case when LO0 ~ 1/3. These will not affect Chapter 7: Multiple Scales Solution 75 the amplitude of the Yo term, though through anti-secularity, they will affect the excitation Co . Of course, they will affect the O(n) terms, and we will see that this will be a noticeable feature of the solution for practical values of the parameters. When the 0(/z2) equations are solved (mostly as a check on the validity of the solution to 0(p) and to provide an error estimate) we will find several new resonances at u>o « 1/5, 1/2, 2, 5, and 7 — but interestingly, not at 1/7. These will not be investigated, as the effects are confined to the 0(ix2) term, and only in small regions. We thus will provide a complete solution to O(n) for Y , and a solution to O(l) for CV, with a nearly complete solution to one more term in each as a validity check and error estimate. 7.2 Case I: Resonance Case, w i t h w0 = 1 + uio\ The equation (7.1.2) becomes Cv + Cv = -2LIIOICV - y?io\CV + ngCv - A H C 3 + DY + BY so, substituting (7.1.5) and (7.1.6) in and looking only at the O(l) terms, we have (7.2.1) a 2 Y C + Y 0 = 0 (7.2.2) dT2 d2C0 dY0 + B d2Yc o dT2 + C0 = D dT dT2 Chapter 7: Multiple Scales Solution 76 These linear equations are solved very easily, as they are effectively uncoupled. Equation (7.2.1) gives Y0 = Ao(Ti,T2,T3,T4)elT + complex conjugate as the most general real solution, where AQ is an unknown (complex) quantity. This form is adopted for computational convenience, as in [15]. Meanwhile, equation (7.2.2) becomes ^ + C 0 = (iD - B)A0elT + cc. Thus, to avoid secular terms in Co we must have Ao = 0. Thus the O(l) solution is (7.2.3) Y0 = 0 (7.2.4) C 0 = B0(r1,7-2,7-3,r4)el'r+ c.c. where BQ is as yet undetermined. The O(n) equations are now * * + y i = _ 2 * * ! L b y ( : . 2 . 3 ) dT2 1 dTdn 1 dT2 and d 2 d d2C0 d2C0 (7.2.5) —1 + C , =-2^-2,^-2,^ dT '{dT J dT dT2 so (7.2.6) y, = A 1 ( r 1 , r 2 , r 3 ) e l T + c.c. Chapter 7: Multiple Scales Solution 77 We thus substitute (7.2.4) and (7.2.6) into the right hand side of (7.2.5). This gives a simple linear oscillator equation for Cx. For this equation to have a bounded solution, we must have the coefficient of elT = 0. The coefficients of e l T are easily obtained, as only one term contains higher frequencies, the cubic term. Substituting (7.2.4) into this term we get = -IBQC + ZIBQBQ6 + cc. dT so, when we set the coefficient of etT — 0 this gives us as our anti-secularity equation dB (7.2.7) -2cjiJB0 + 2CTI.BC, - 2i—-+ igB0 - t • + {iD- B)A} =0 and equation (7.2.5) becomes a simple oscillator equation with a single term of frequency 3 on the right hand side, which is easily solved, giving (7.2.8) C1=B1{TUT2,T3)eiT-liiB*ei-ST + cx. Equation (7.2.7) connects Bo and A\, but we need one more equation. We look at the 0(n2) equations, and the first of these will provide our required second equation. The first 0(fj,2) equation is d2Y2 v _ d2Yx d2Yx — + Y 2 - - 2 o 1 — - 2 - ^ - + sC0 Chapter 7: Multiple Scales Solution 78 so the anti-secularity equation is ' dA\ (7.2.9) -2i—J-+2o1A1-rsB0 = 0 on which leaves Y2 — A2{T\,T2)elT + cc. as in the 0(p) case. Remark The quasi-steady term plays no part as yet. We will see that the O(p) terms are determined in the resonance region completely independently of the quasi-steady excitation. This makes physical sense as we would expect the vortex effects to dominate in the resonance region. If we put equations (7.2.8) and (7.2.9) in real form, with A \ = |aie l* J and B0 - \b0e1^ where ax = ax (r 1 ; T2, T3), b0 = b0(T1,T2,T3,T4), fa = <pi(rl5 r 2 ,r 3 ) , and 0o = 0o(?"i,7-2,T3,r4), we get (7.2.10) b 0 ^ + (a, - W l ) 6 o - ^ s i n ( f c ) - ^  cos(fc) = 0 OT\ I 2 3_ dd> 1 (7.2.12) a , - ^ -f-ffiO! + -560cos(ei) =0 (7.2.13) - - ^ - - - S 6 0 s i n ( f i ) = 0 OT\ 2 where Z,\ = 4>\ — 0o-Remark These equations are singular when a\bo = 0, due to the transfor-Chapter 7: Multiple Scales Solution 79 mation to real form. This necessitates special handling for the stability of the zero solution. 7.3 Solution of the O(n) equations We wish to solve equations (7.2.10)-(7.2.13) explicitly; unfortunately, this is not possible. However, we can find special solutions of these equations, which will be enough for our purposes. We look for limit cycle or steady-state solutions. We remark that a steady-state solution of equations (7.2.10)—(7.2.13) is not in general possible, as only the phase difference £i appears in the steady equations. This means that when the T\ derivatives are zero, we get a system of four equations in three unknowns, which is in general inconsistent. Instead of requiring each of 4>\ and ipo to be steady, we can require that their difference fi be steady. This can also be viewed as looking for a limit cycle solution where the frequency of <f>\ and tpo is the same on the rj-scale. This leads to a consistent set of four equations in four unknowns. By putting <t>\ = STI + (f>(r2,7-3), V'o = &T\ + V,o(7"2> T3, Ti)i the phase difference fx = <f>\ — xjj0 is independent of T\. If further = | ^ = 0 our equations become (7.3.1) 60(0-! + S - U l ) - ^ sin(e1) - ^ c o s ( £ i ) = 0 Chapter 7: Multiple Scales Solution 80 gbo (7-3.2) 2 axD . a,]B . .„ . + -^-cos(ei)--^-sin(ei) = 0 (7.3.3) G l (a +S) + ~sb0 cos(ei) = 0 (7.3.4) -^6osin(ei) = 0 These equations are easily solved. Note that A\ = Bo — 0 is a solution of the original equations (7.2.7) and (7.2.9), so we may restrict ourselves here to looking for solutions with at least one of a\ or 60 nonzero. Note however that if a! =0, then (7.3.3) and (7.3.4) together imply that bo — 0 also; likewise, if b0 = 0, then (7.3.1) and (7.3.2) together imply ax - 0, if B2 •+ D2 ^ 0. Thus we may assume henceforth that neither ai nor bo is zero. Thus (7.3.4) gives £i = 0 or £i = ir, and (7.3.3) then gives (7.3.5) o1 + 6=^coS(f1) = T ^ b o 2ai v ' 2a and we are left with the two polynomial equations (7.3.1) and (7.3.2) for the two remaining unknowns ai and bo. To keep track of the signs, we leave cos(fi) in the equations. With (7.3.4), (7.3.1) becomes a quadratic equation for bo/a\, with solutions (7.3.6) ^ ^ ^ i l y C f T S ai scos(^) s v whenever this is strictly positive. Thus for each £ 1 ? we have two possible solutions Chapter 7: Multiple Scales Solution 81 for bo/a\. Lastly, (7.3.2) now becomes (7.3.7) 1 + whenever this is strictly positive. Note that if B < 0, this ratio 60/^1 is never zero throughout the range for u)\. If, however, B is zero, one can show that when u»i = (7.2.10) — (7.2.13). We ignore this exceptional case. Thus we have at most four different limit cycle solutions, for any given set of parameters, and one free parameter (either o\ or <5, so long as (7.3.4) is satisfied). The fact that we have found a solution only at a limit cycle means that we must take care that the higher-order time scales do not disturb this limit cycle. Thus we must investigate the effect of the next terms on the solution found at this stage. Also, we are concerned with the stability of the limit-cycle solution found in this section. The previous remarks noted that we would like to see the effect of the higher-order time scales and smaller terms on the solution, but with the stability question we are more concerned with the effects on the limit-cycle solutions of perturbations of the first terms, perhaps caused by the effects of the higher order terms. Thus we first look at the linear stability of the limit-cycle solutions. O(n) that there is no steady-state or simple limit-cycle solution to the equations R e m a r k We must investigate the r2-scale to see if this is a consistent solution. Chapter 7: Multiple Scales Solution 7.4 Stability of the 0(/z) solutions Noticing that we can combine equations (7.2.10) and (7.2.12) to get 82 (7.4.1) + Wl + 1 1 cos(£i) + -i-sm(ei) =0 5ri \2a\b(j 2aj6o / v""y 2oi6o and that = <S — 6 = 0 at the limit cycle, we can investigate the stability of the limit cycle by linearizing the equations (7.2.11), (7.2.13), and (7.4.1) about the steady state of this compressed system. The signs of the eigenvalues of the 3 x 3 Jacobian determine the linear stability of the system in the usual fashion. The Jacobian is (7.4.2) Jf(ai,b0, fi) f£>cos(6) 1 - 3 ' 0 - | 6 0 0 c o s ( £ i ) "\ -|oiBcos(^) • n V t e * - 2 t ) c o s ^ ) ("air*+%)««(&) - W ^ D c o s ^ ) and then, with the usual linearization about the steady state (oj,60, fi), d Aai A6 0 Mi Aai A6 0 A6 + higher order terms. This analysis fails if ai6o = 0, due to the singularity in the transformation to real form. To analyze the stability of the zero solution, we must go back to the original (complex) form, equations (7.2.7) and (7.2.9). Linearizing about (Y,C v) = (0,0) we get 2 -f h. o. t. d Bo. lO\ L 2 Chapter 7: Multiple Scales Solution 83 and the real part of the trace of this matrix is g/2 > 0, so at least one eigenvalue must have positive real part; and thus the zero solution is unstable throughout the resonance region. Remark This result is consistent with the experimental phenomena we are attempting to model. Notice that the simple quasi-steady model, for example, does not predict the instability of the zero solution in the resonance region. Of course, as to this order our model is indistinguishable from the (generalized) Hartlen-Currie model, the Hartlen-Currie model does predict this instability. Remark The solution to O(l) for Fo is zero, and we cannot establish the stability of this solution in the normal fashion. Looking at nearby solutions and investigating their relationship with the zero solution is not a valid procedure in this case, because there are no other solutions, nearby or otherwise. This is the mathematical phenomenon of rigidity, and in one sense it means that the O(l) solution is stable, in that there is no other. However, this is less satisfactory than, say, asymptotic stability, because it is not clear what happens physically when the 0(/Lt) solution becomes large. Thus we are concerned with the stability of the O(n) solution, including the zero O(M) solution, on the assumption that this is the physically relevant quantity. Chapter 7: Multiple Scales Solution 7.5 S o l u t i o n to 0(n2) 84 We wish to determine A2 and B\, and to ensure that the T2-scale does not affect the first term solution Ax and Bo. The second terms may be important in the case of larger n (i.e. oscillation in water), and should also help to smoothly join the resonance and non-resonance regions. We look first at the second 0(fi2) equation: d2C2 dT2 + C2 = -2uXCX - OJ2C0 - 2ox d2cx d2d [Pi + 2a2) d2C0 dT2 4CTI dT2 dTdri d2C0 d2C0 n d2C0 dTdn dr2 - 2-dTdr2 + 9 + D + B dC\ dCo dCo ~df~+ °L HT + "5r7 (dCpX {dT) dCx dC0 dC0 dT dT drx dY2 dY, dYx + — h Oi dT drx d2Y2 _ d2Yx + 2 dT2 dTdrx dT + 2ox d2Yx dT2 and as dCo) dCi dT j dT iB0eiT + c c . ) ( iBxexl + ^B'^e1'3'1' + c c JT >3_t 3T i • 2B0B0Bi + IBIBX + ^BQBI ) elT + other frequencies our anti-secularity equation becomes (7.5.1) dB 2% + (2ox - 2UJx)Bx + igBx drx Chapter 7: Multiple Scales Solution 85 - 3 7t(2£oB 0£i + BoBi) - ll2B^B20 o + (iD - B)A2 - u\B0 + (o-i + 6){igB0 - 9nB2B0 + [iD -2B)Al) + 2 t — - + [p\ + 2o2 + + o~ 2)£ 0 C7T2 = 0 where we have used — SBo and = 6A\, which is true at the limit cycle. Remark This equation is a nonlinear partial differential equation, in the vari-ables T\ and T2, which again we cannot solve in general. However, we will show that we can satisfy these equations by separately setting the quantities in square brackets to zero. Note that this equation can be split up in several ways in a search for special solutions. We will also need the first 0(fiz) equation: d2Y3 dT2 + Y3 = -2a-d2Y 2 2B2Y2 - 2 dT2 dTdrx  d2Yj _ (P% _ d2Yj dr2 ~*°XdTdTX dTdr2 iv, j d2Yx [of + 2o2) 32Y0 dT2 dTdr3 Chapter 7: Multiple Scales Solution which gives as our anti-secularity equation 86 (7.5.2) -2i .dA0 dr3 - 2i^ + (o\ + 2a2 + 40-iS + 62)AX O T 2 + •dA2 -2i—— + 2oxA2 + sBi + irxAx Again, we split this equation up into the equations in square brackets and require that they be zero separately. We note first that the two f2-scale equations (7.5.3) (7.5.4) -2t'^^ + yo\ -w\ + 2o2 + Aoxb + S2jAi = 0 dB -2i~of- + ( °i ~ w i + 2 c r 2 + 4oi6 + 6* ) Bo = 0 are easily solved, and imply that ^ = -^r(4>\(T2) — xpo(T2)) = 0 and that = -Q^ — 0, so the 72-scale has no effect on the first terms, regardless of the choice of ai, 6, or 02. Thus we can get a consistent solution from this separation, which justifies ex post facto the separation used. Notice that the r3-scale does not affect the solution at all in this separation, as AQ = 0. Now we look at the system formed from the third set of brackets from (7.5.2) together with the first set of brackets from (7.5.1). We try to solve this system for By and A2. We look for special limit-cycle solutions as before, and in fact insist that the new terms have the same Chapter 7: Multiple Scales Solution 87 ri-frequency. Thus we set 2 Bi = \bi(Ti,T2,T3)e^>^>^+6^ where the 6 is the same as in the first terms obtained. For notational convenience, we define £2 = 4>2 — , — V>o - ^lj and u s e the shorthand notation sx = sin^), ci = cos(fi), Sd = sin(V>d), s2a- — sin(2^<i), and similarly for sin(f2) and the other phase angles. Then, what is left of (7.5.2) becomes in real form da.2 d(f)2 (7.5.6) s2— r c 2 a 2 — \-(01 + 6)c2a2 OTi OTi 1 t 1 + -sbi - - r i a i c i s d = 0 (7.5.7) - C 2 — + s2a2- h (ai + 6)s2a2 OTi OTi 1 - - n a i l e d = 0 where we have used the fact that £j = 0 or 7r. Thus, at a 7"i-steady state, (7.5.8) (CTI + S)c2a2 + -sbi — ^ r ^ j C i s ^ = 0 (7.5.9) (ox + 6)s2a2 - ^ n a i C j C d = 0 This allows us to eliminate £25 and when oi + <S ^ 0 we have (7.5.10) a2, = 4 ^ * + s y ({riaiCiSd - sbi)2 + ( r i O j C ^ d ) 2 ) . Now we examine the first bracket in (7.5.1). We use the symbolic computation lan-Chapter 7: Multiple Scales Solution 88 guage REDUCE [ll] now as the equations are getting tedious for hand computation. By REDUCE, the equations in real form are (7.5.11) 6, ^  + (c^  + 6 - ux)bx + libls2dbi 1 1 ^  Ba2c2 Da2s2 = 0 2 2 and (7.5.12) _ _ i + _ -lbl - - 7 f c 2 C 2 d j 6 i - cd (^bo - \sbo - ^Dcxax^j (ai + 6) ( 1 9 + sd ( - -w 2 6 0 + ^l2bl - B(ox + 6)cxax H — D a 2 c 2 — -Ba2s2 = 0. We can use (7.5.8) and (7.5.9) to eliminate both f2 and a2 from these equations, at Chapter 7: Multiple Scales Solution 89 a rj-steady state. Putting for notational convenience (7.5.13) 9i = 1 3 2 29 ~ 4 l b ° 92 = 1 2{o1 + 6) Pi = o\ + 6 — ui P2 = P3 = 1 2. 9 Pi = ( f i - S - j * * . PS = 2 P& = -ID, 2 ' ..2j.5 then (7.5.11) and (7.5.12) become, at steady restate, (7.5.14) pi • bi + p2 • s2d • h + (pz - q2PQriaic)cd + (P4 + <l2Phriaic)sd - q2P5sbi = 0 (7.5.15) qi • bi - p2 • c2d • h - (P4 + q2PhT\aic)cd + (P3 - q2P&riaic)sd + q2P&sbi = 0. These equations are nonlinear in but we may solve them by forming the combi-nations Cd x (7.5.14) + S d X (7.5.15) and Sd X (7.5.14) - c ^ x (7.5.15), which because of the identities C d S 2 d — $dc2d = sd a°d Sd52d + cdc2d = cd a r e linear in Cd and s^. Chapter 7: Multiple Scales Solution 90 From here we proceed to a complete solution. Making these combinations gives (7.5.16) (pibi - q2p5sb1)cd + (gj&i + p 2 + q2P<5sbi)sd = ~Pz + QiP&ria^i (7.5.17) (~q\b\ + Pi - q2Pesbi)cd + (pxbx - g2p5sbi) sd = -PA - q.2Psriaicx. Remark The solution of these linear equations for cd and sd in terms of &i and the first-term solutions allows us to set up a single equation in the single remaining unknown bi by noting c\ + s\ = 1. On solution of this equation for 6i, we then use the linear equations to determine cd and sd and hence xpd, and then we can use (7.5.8)-(7.5.10) to determine a2 and £ 2 . Putting 4^.11 = Pi ~ Q.2P5S M2 = Qi + 92P6* A21 = -A12 A22 = AU Bu = ~Pz + q2p&rxaxcx B22 = -PA - Q2PbT\aiCi Chapter 7: Multiple Scales Solution 91 then the solution of the system (7.5.16)—(7.5.17) can be obtained by e.g. Cramer's rule: Bu Ai2bi + p2 B22 A^bi -A Aubi AX2bi -r 12&1 + P 2 Aub Aubi Bu -Ax2bx +p2 B22 • P2 1 Aubi AX2bi+p2 -Ai2bi+p2 Aubi and our last equation, for 6i, is c\ + s\ = 1. By inspection, we see that this single equation for 6j is a quartic equation, so an analytical solution is available if desired. It makes better numerical sense, however, to use a more general numerical method to find the real positive roots, as the analytical formula can be unstable numerically. Remark Strictly speaking, we should calculate the stability of the 0(/J, 2) terms in a manner similar to the process used for the O(n) terms. However, we shall see in the later section on the solution in the nonresonance region that the stability of the higher-order terms is effectively determined by the stability of the first terms calculated. We shall assume that the same situation holds in the resonance region. This is reasonable, as the solution to this order will only be used for error-checking, and if the solution to this order does not differ too much from the solution to the previous order, then we can think of the second-order terms as a perturbation of the first-order solution, and rely on the first-order stability analysis. If on the other Chapter 7: Multiple Scales Solution 92 hand the difference between the solution to the two orders is large, then we can no longer rely on the previous stability analysis. However, if this is the case, then the validity of the solution to the previous order is then in doubt as well, and a stability analysis of the second-order terms would tell us nothing useful. In Figure 7.5.1, we see a demonstration of this effect. For u>o < 1.04, we have good agreement between the solution to one term and the solution to two terms. Since the stability analysis for the first term solution shows that this branch of the solution is stable, we can conclude that the solution in this region is accurate. However, we see at or near u>o = 1.04 the beginning of large oscillations in the two-term solution. This is not physically significant, but merely signals the possible end of the region of good accuracy for the one-term solution. Recall that here the method of multiple scales is expected to give an asymptotic series as the solution of the model equations. In an asymptotic series, taking more terms does not always increase the accuracy obtained: in fact, the usual case is that there is an optimal number of terms to which to take the series to for minimal error, and if more terms than this are taken, the error begins to grow. Thus when we see good agreement between the solution to one term and the solution to two terms we feel confident that the true solution is represented well by the solutions presented. However, when the solutions do not agree, we have less confidence in the two term solution; the one term solution may still be adequately accurate. Chapter 7: Multiple Scales Solution 93 Here, we can see that the solution to the first term is sufficient up until CJQ = 1.04, as the true solution should be between the solution to one term and the solution to two terms. After the solution to two terms starts to oscillate, however, we have no guarantees of the accuracy of the solution, and the true solution of the model equations may follow the one term solution (as it can be expected to for some range after u>o — 1.04) but cannot be trusted. Eventually, the one-term solution becomes very large, and this is a further indication of the loss of accuracy. This loss of accuracy arises out of the breaking down of the assumptions about the size of Y\, which is becoming 0(1) rather than O(n). There are some experimental values from [l] also plotted in Figure 7.5.1 for comparison purposes. The solution agrees with the general upward trend of the data, though it overpredicts the size of the amplitudes. Recapitulation In terms of the original (nondimensional) variables, the solu-tion obtained so far may be written as Y = nai cos [(1 + p(ox + 6) + n2o2 H )t + <pi] + n2a2cos [(1 + n{oi + S) + ii2o2 + •••)* + 4>2] + 0(fi3) Cv = b0 cos [(1 + n{ox + 6) + p2o2 + •••)* + Vo] + \ibx cos [(1 + n(ci + S) + n2a2 + •••)* + xpi] + 0(n2) where we may take <px — 0 because of the autonomous nature of the model equations, Chapter 7: Multiple Scales Solution 94 >-0.25-1 0.20 0.15-0.10 0.05-n = 4.7x10~4 a = 0 . 1 3 X U J J 1 D = 0.855/u 0 B = - 2 . 3 5 / u 0 2 C v - 1.40 A = 4.87 A = 4.21X102 3 4 A = 1.70x10 5 5 A ? = 1.94x10 / 0.00 • / a • a • • • Legend Sfable_First ^rmJSolution _ Stable Second Term Solution • BGMP Experimental Data 1 1 1 1 1 1 1 1 1 1 1 I I 0.80.850.900.95 1 1.05 1.10 1.15 0 Figure 7.5.1 Solution to O(n) and 0(n2) in the Resonance Region. and all the other parameters (except 02, which we are free to choose) have been determined in the previous sections. Note that the parameter 6 appears throughout only in the combination ox + 6, and thus could profitably have been omitted. This Chapter 7: Multiple Scales Solution 95 was not evident a priori however, so 6 was left in the analysis. At this point we may set it to 0, however. Notice also that the effect of o2 is not felt on the r2-scale, as CT2r2 occurs in the solution for il>o(T2, Tz, TA) and cancels with the occurrence of a2ri2t in the argument to 6ocos(-). Any effects of the choice of cr2 are thus confined to higher order terms, so we may as well take cr2 = 0. The nature of the solution is that of a limit cycle in four dimensional phase space. We can easily determine the stability of this limit cycle, through the stability analysis of the first order solution. 7.6 Case II: Nonresonance Case, with u>0 ^ 1 This section will complete the solution to O(p) in Y and to 0(1) in Cv in the nonresonance case, and show where the superharmonic and subharmonic cases arise from. We will investigate the latter cases in the sections following. Here the O(l) equations are, almost as before, (7.6.1) ^ + y ° = ° (7.6.2) ^+ulCo = D?Xl + B^ which have solutions (7.6.3) Y0 = Ao(TUT2,T3,T4)eiT + cc. (7.6.4) C 0 - Bo(ri,7- 2,r 3,T 4)e ,' u"' : r + ^ D ~ f ^ A0elT + c c u0 - 1 Chapter 7: Multiple Scales Solution The O(n) equations are then 96 (7.6.5) and (7.6.6) d2\\ dT2 d2d dT2 d2Y0 d2Y0 dT2 dTdn . d2c0 d2c0 + 9 + D + B — 1 dT dYi dT d2Y, dT2 dCp dT ^ dY0 ^  dYQ d2Y0 + 2CTJ + 2 d2Y0 dT2 dTdn and our first anti-secularity equation is (7.6.7) .dA0 2CT!^O - 2 t — — = 0 on giving (7.6.8) A0 = A0{r2,T3,T4)e-icTiTl after which (7.6.5) gives (7.6.9) Y\ = Ai(Tl,r2,TZ)elT + cc To get the anti-secularity equation for (7.6.6), we must set the coefficient of etw"T to zero. For notational convenience, put v — IUJQBQ and A = — (D-\-iB)A0/{u0l — 1). Chapter 7: Multiple Scales Solution 97 Then, using (7.6.4), 3 — v e 3 > 3 u > „ T 2-j- iwi,T + 3 „2 A <,i(2u, ( , + l ) T + 2 l / J ? X e i T + „2Je ,t"(2w()-l)T + 3 [i,A V'( w « + 2 > r -f 2i/AA e^-r + A2i/e , i ( w „ - 2)r + A3e 3„i 3T + 3A 2Ae l T + ex. We wish to investigate which values of u>o give rise to resonance. Thus, we look at the frequencies present in the equation (7.6.6) after (7.6.10) has been substituted in, and ask which terms have frequencies that resonate with LJ0. For different values of LOQ, there may be different terms entering in to this process. For example, if u>o = 1 + O(fx), then 2wo — 1 = UQ + O(n) and this causes a resonance. By inspection of the equation, there are four different cases: OJQ « 1, which has already been handled in the previous sections, u>o « 1/3, UQ « 3, and lastly, W Q ^ 1, 1/3, or 3, the nonresonance case. If wo = 1/3 + 0(/x), this is the phenomenon of superharmonic resonance, and the —(2wo — 1) term in (7.6.10) goes into the anti-secularity equation here, resonating with u>o, and the 3wo term will later resonate with 1. If UJQ = 3 + 0(H), then the term at frequency 3 will resonate with u>o, while later the UJQ — 2 term will resonate with 1. We will see later that the subharmonic resonance is the more important of the two for our models. In this section, we assume henceforth that u>0 56 1/3 and that u>0 3. Under this last assumption, the Chapter 7: Multiple Scales Solution anti-secularity equation for (7.6.6) becomes 98 (7.6.11) dBo . 2 . -2iu0— V \2OXUJ0 + lUogjBa - 7(3i/2z7 + 61/AA) = 0 which leaves in (7.6.6) d2C (7.6.12) + ulC, = [ (iD - B)AX + gX 7(6//]7A + 3A2A) e iT 1 I /3 e t.3W | ,r + 3 i /2 A e t(2 W„ + l ) T + 3i / 2 Ac , "( 2 w »- 1 > r + 3i/AV<w"+ 2>T + 3^AV ( w ' ' - 2 ) t + A V 3 T | + cc. which is easily solved, giving (7.6.13) C i = B 1 ( T 1 , T 2 y " » T + K l e i T + K 2 w o _ i e « ( 2 - » - 1 ) T + ^ ( ) + 2 e ^ + 2 ) ^ + CC. where KS = cs/(w2 — s2), with C5 equal to the coefficient of elsT in (7.6.12), for Chapter 7: Multiple Scales Solution 5 = 1, 3C J O , 2u>o + 1, 2u>o — 1, OJQ -f 2, W Q — 2, and 3. 99 Remark The nonresonance case is more complicated than the resonance case, in that there are more frequencies present in the O(l) and 0(/z) terms. However, this presents no real difficulty, just a little more work. We solve the anti-secularity equation (7.6.11) by splitting it into real and imag-inary parts: putting BQ — \b§tx^", we have (7.6.14) (7.6.15) dib0 2 unb0— h OiL00b0 = 0 dbo - h vogbo 2 - 1 3 3 , 3 ^ 3u0{D2 + B2)a2b0 8 W° 6° + 4(u2 - 1)2 = 0 which has solution bo — 0 or (7.6.16) (7.6.17) i>0 = -OiUJoTi + tl>o(T2,T3,T4) CYl)\/h bo 0 - K(T2,T3,r4)e-h^ if /i > 0 where (7.6.18) , ,r , , 2(£>2 + B 2) 2. G y ( ) u ; o l u ; o ~~ and K ( r 2 , 7 3 , r 4 ) is an arbitrary constant of integration on the rj-scale. Chapter 7: Multiple Scales Solution 100 Remark If h < 0, then it is easily verified that all solutions of equation (7.6.15) decay exponentially to 0. This shows that if a,Q is too large, then the only stable solution for bo, the 0(1) amplitude of the Strouhal frequency component in the wake, is zero. This occurs only in the resonance region, when OJQ ~ 1. This corresponds to the entrainment or lock-in of the wake frequency to that of the body. Remark We see that equation (7.6.18) implies that for any fixed T2,T3,T4, bo —• Cy0\/h, if h > 0. This tells us that the excitation, to first order, is determined wholly by the r -^scale. We must check that the higher-order equations are consistent with this solution. We must yet determine ao(r2, T3, r 4), <PO{T2,T3,T4), and IPO[T2,T3,T4) to complete the solution to first order. To do this, we look at the first 0(/z2) equation: ( 7 - 6 - 1 9 ) + F 2 = -2<xi-5=5- -2-dT2 * 1 dT2 dTdti d2Y0 A d2Y0 d2Y0 _2d2Yo dr2 dTdT2 dY0 dYo.a (dY0.s ( 8 Y 0 r + sC0 Chapter 7: Multiple Scales Solution so to avoid secularity we must have 101 (7.6.20) 2i dA] +2axAx + (o\ + 2o2)A0 - 4o\A0 9 .dA0 + olA0-2i—^ + i\r\A0 - 3r3AlA0 + 10r5AlAl - 35r 7^^Io (iD - B) A + s -tCTl T, 0 and to avoid secularity on the rj-scale in this equation, we must have the coefficient of e~t<7lTi equal to zero. Remark Contrast this with the resonance case solution, where we had to choose how to split up the higher-order resonance equations. Here we automatically have two different equations on the two different time scales, which gives much greater confidence in the solution. Thus we have the following equations: dAi (7.6.21) -21—^ + 2(7^=0 Chapter 7: Multiple Scales Solution which has solution 102 (7.6.22) A1{TUT2,T3) = ^i(r 2 ,r 3)e 1 ( 7 and the other equation is (7.6.23) 2t .dAp dr2 + 2{o2 -o\)A0 -sB ul - 1 A0 + i\riAQ - 3r3i4^i40 + 10T5AIAI - 35r7A^Ap sD + t 0 or, in real form, with AQ = \ape^°, (7.6.24) (7.6.25) where (7.6.26) a 0 d<f>o dr2  dap dr2 + [o2 -= /(ao) /(ao) = ap ~2 sB 2 K - 1) )a 0 = 0 sD 5 4 35 6  + 8 r 5 a ° ~ 6 4 r ? a ° Remark We can solve these equations completely, though in the general case our solution for ao is in an implicit form. In the special case rs = r-j — 0, we can provide an explicit solution for ao also. It is interesting to compare these equations with the corresponding equations we get from the simple quasi-steady model due Chapter 7: Multiple Scales Solution to Parkinson and Smith [20]: 103 (7.6.27) dao _ ao ~d72 ~ T 3 o 5 4 35 o ri - - r 3 a 0 + - r 5 a 0 - ^r7a0 which differs only in the linear term. This means this model is precisely as easy to solve as the quasi-steady model is, although the higher-dimensionality of the problem complicates the geometric picture of the limit cycles. We will also see later that equation (7.6.25) is unaffected by the subharmonic and superharmonic cases, thus confining their effects to the higher-order terms. Before we proceed to solve the anti-secularity equation, we exhibit the form of the solution for Y2 from what is left of (7.6.19): (7.6.28) Y2 = A2(TUT2)eiT + l 3 e i 3 T  + lsei-ST + ljei.7T + l U o e i ' U a T + cc . where A3 — —2 h = i-£[r3 - 5r5A0A0 + 21r7A20A0] o A5 — ts = i^[rs-7r7A0A0] A7 l7 — i — r7. 48 / - *Bo w" ~ 1 - ul We first solve the anti-secularity equation (7.6.25) in the important special case Chapter 7: Multiple Scales Solution 104 when Ah = M = 0, which is often observed for cylinders in turbulent flows. Our equation becomes (7.6.29) ^ = /(a 0) = \a0 sD 3 2 r\ + —2 - - r 3 a 0 wg - 1 4 In this case, since the equation is separable, and the resulting implicit equation for ao(7"2) is solvable (which it is not in the case A^,A7 ^ 0), we can get a complete solution, and this gives extra insight into the higher-order polynomial cases. The solution in this case depends principally on the sign of the linear coefficient, 2/'(0) = ri -f sD/{LO 2 — 1). If this is negative, then it is easy to see that all solutions of (7.6.29) decay exponentially to zero (on the r2-scale, for any fixed r 3 and r 4 ) , and any initial conditions. If the linear coefficient is zero, the solution again decays to zero for any fixed 7-3 and r 4 , but in this case the decay is algebraic. If the linear coefficient is positive, the solution can be written / 2/'(0) (7.6.30) a 0(r 2 ,7- 3,T 4) = ' v ; f r 3 - K ( r 3 , r 4 ) e - 2/'(0 ) r 2 where as before K is an arbitrary constant of integration on the TX-scale. We see that for all finite values of K and all fixed values of r 3 and r 4 that the solution tends exponentially to a nonzero steady state. The zero solution corresponds to the case of infinite K; we should really go back to the complex form to investigate the zero solution, however, to avoid the singularity introduced in the transformation to real form. When we do this, we find, as expected, that if 2/'(0) > 0 then the Chapter 7: Multiple Scales Solution 105 zero solution is unstable, and likewise when it is negative the zero solution is stable. Thus in the case of ^ 5 = A7 = 0, we have a complete description of the first terms of the solution to the model equations. It is important to note that all nonzero solutions tend to the single nonzero solution (an 'orbital attractor' in mathematical dynamics jargon), the steady state given by K = 0 or (7.6.31) a0 = f Remark In the case D = 0, this reduces to precisely the quasi-steady solution. Recall, though, that the solution here is valid only outside of the resonance region. On closer inspection of the solution given above, we note that for C J 0 « 1 the value of ao can become arbitrarily large. However, before ao gets too large, we see by equations (7.6.17) and (7.6.18) that 60 will g° to zero if a0 is too large. We simply have to use our judgement as to when the solution given above is valid, as it is outside the resonance region. One could wish for a more clear-cut division of the solution into regions, but it is usually clear from the regions of overlap of the solutions just how far each region's solution may be pushed. Remark Note that the steady states of the solution and the stability of these states provides a complete description of the long-time behaviour of the solutions to the model equations. We now have a complete solution of the model equations to O(l), in that 60 and a0 are both known, in the case A$ = A7 = 0. We next Chapter 7: Multiple Scales Solution 106 o.i-Legend A PotynomM :< Sfebta Root* • Un»to±4. Roots Figure 7.6.1 Location and Stability of the Steady-State Amplitudes. Case I: /'(0) > 0. investigate the solution in the case of nonzero As and A7. Recall from equation (7.6.26) that da0 ,, , 1 sD 3 2 5 4 35 G r l + — 7 ~ T r3Go + o r 5 ° 0 _ 7 7 r 7 a 0 - 1 8 64 so the zeros of /(ao) are the steady-states of (7.6.25), and the stability of a steady state aj is determined by the sign of /'(^o) from the usual linearization technique. Chapter 7: Multiple Scales Solution 107 0.5 Legend ;< Stobt* Root« D Un»tobt« Roots —I 1 1 1 1 1 i i 1— O.t 0.2 0.3 0.4 0.S 0.6 0.7 0.8 0.9 -1 "T 1 1 1.1 12 Figure 7.6.2 Location and Stability of the Steady-State Amplitudes. Case II: /'(0) < 0 In particular, the zero solution is stable if and only if (7.6.32) 2/'(0) = n + sD Ai{U-U0) + U2D{u0) < 0. It is interesting to note that this, together with the number of real positive roots of /(ao), completely determines the stability of each real root. The possible situations are summarized in Figures 7.6.1 and 7.6.2. Figure 7.6.1 shows a graph of a typical polynomial of the type presented in equation (7.6.26), with /'(0) > 0. There is always a root at 0, and there is always at least one positive root with /'(flo) < 0 Chapter 7: Multiple Scales Solution 108 as the highest-order coefficient in the polynomial is negative. There may or may not be another two roots present, depending on the values of the other coefficients. The roots with /'(a^) < 0 are stable, and the others are unstable. Figure 7.6.2 shows the analogous situation when /'(0) < 0. In this case it is possible that there are no roots other than 0. This completes the solution of the equations to O(l). In Figure 7.6.3 we present a sample solution of the model equations to this order, and compare this solution to data from [l]. Note that, to 0(1), the solution in the resonance region is zero, but that outside the resonance region, agreement with the data presented is quite good. In this low-damping low-turbulence case, the quasi-steady model predicts a nonzero amplitude starting from UJQ = Uo/UT — 0.63. This model on the other hand predicts that nonzero amplitudes will occur only after the resonance region, which is what is physically observed. Remark To this order, solving the model equations is precisely as easy as solving the galloping equation. The solution is zero in the resonance region (to first order) and the steady states outside this region are given by the roots of the cubic (in OQ) polynomial (7.6.32). To this order, the subharmonic and the superharmonic resonances do not enter into the solutions. These resonances play a part in the next order terms. Chapter 7: Multiple Scales Solution 109 0.9-0.8 0.7-0.6 >- 0.5-0 .4-0.3-0.2-0.1-0 n = 4.7x10 a = O.UXUJJ 1 D = 0.855/o>0 B = -2 . 3 5 / u 0 2 C v = 1.40 T 0 A 1 = 4.87 A = 4.21X102 3 4 A = 1.70x10 5 5 A ? = 1.94x10 / ;-. / • ' / ;..y Legend Wake ^ scjllator^Mo_de[ O Low Damping Data [ 1 ] ' i ' 4 - 1 '— i 1 1 1 1 1 1 1 0 0.5 1 1.5 2 2.5 3 3.5 4 4.5 5 0 Figure 7.6.3 Solution to O(l). cf [l] Chapter 7: Multiple Scales Solution 7.7 Nonresonance Solution to 0(H) 110 The first 0(H3) equation is, by REDUCE, in the case o\ = 0, ~df^ + Yz- ~2dfdTy ~2°2^f2~~2dfdT2 (7-7-1} d2Y0 d2Y0 + s • C\. and our anti-secularity equations are thus in the case CJO 76 3 and wo 7^ 1/3 and taking ox = 0 (7.7.2) - = 0 (7.7.3) - 2 ^ = 0 (7.7.4) - 2 t — - = -20-3^0 -2" + » r j ^ ! - 3r 3 [ i 4 0Ai + 2 ^ 0 ^ o ^ i - 7r7[l5>l0yio^i + 20A30A30AX} Now (7.7.2) and (7.7.3) are trivial, and we may find the steady-states of (7.7.4) in the following manner: Put <{>d — <t>o — 4>\\ then on division by e^S (7.7.4) in real Chapter 7: Multiple Scales Solution form becomes i l l d(f) 1 772 (7.7.5) - — — = -sin(20d)m1 ( -Dcos<pd + Bsin<f>d O T 2 2 di - Oz [ — ) COS </>d \ a l J and (7.7.6) = -o- 3a 0 sin <pd O T 2 1 / , x 1 - -miai cos(20d) - - o i m 3 m 2 I —I? sin (j>d — B cos where (7.7.7) m i = " / 3 f l o + : r 5 f l o - ^ r r 7 f l o 4 4 64 3w^6ga0 3(£>2 + B2)al (7.7.9) m 3 = r, + T - , - ^ - - r 3 a 0 + ¥ r 5 a 0 - - r 7 a 0 . Now, denoting cos by c<£, sin<^ d as 5^, and similarly for the other angles, and noting that mi — m 3 = /(ao) = 0 and that mi + m 3 = /'(ao), and putting Pi = a3ao — m2D, we get at steady state (7.7.10) pi • cd - sd(m2B - ra^iCrf) = 0 and (7.7.11) p i • sd + cd(m2B - m1a1cd) = 0. Chapter 7: Multiple Scales Solution 112 Now, multiplying (7.7.10) by Cd, (7.7.11) by Sd, and adding, we get P i ^ + c2,) = 0. Thus pi = 0 or CT3 = m2I?/ao, or the appropriate limit when ao = 0. Similarly, multiplying by — Sd and Cd and adding, we get (s^ + c2d)(rri2B — m-iaiCd) = 0, so we have an equation for the product a\Cd- This is sufficient, as by our use of <73 we have shown that 4>\ = — <f>d is now a free variable. Then we can choose the steady state solution as sin <f>d — 0 by choice m2JB (7.7.12) o! = so Y\ — a\ cos(T + <f>d) = o-i cos <f>d cos(T) if we take <f>o = 0 by the freedom to choose a time origin. Remark Note that mi = /'(ao), and a simple stability analysis shows that ax is stable if and only if the corresponding ao is stable. This consistency gives confidence in the results. Note also that the choice of 4>d = 0 or 4>i = T is immaterial, as the sign will cancel out in the Y\ term. 7.8 Subharmonic Solution to 0(/x): w0 = 3 + /zw3 Equations (7.6.1) through (7.6.10) are unchanged in this case, but the anti-secularity equation for (7.6.6) is not (7.6.11) but rather, using uiQ = 3 + /xu>3 and Chapter 7: Multiple Scales Solution Tl = pT, 113 dB (7.8.1) -2iu!0— h 2o-]CJo-Bo = -iu0gB0 + 7 which has the new term r)X3e~lu'"Tl, which is included because the e l Z T term res-onates with UJQ. This equation is autonomous if and only if one of ao = 0 (which implies that A = 0) or (7.8.2) —ZO\Ti — = 0. So we naturally take o\ = — w3/3, compared to 0 in the nonresonance case. This is immaterial in the case ao = 0. Then, D + iB A — 2 — 7 - ^ 0 ( ^ 2 , 7 3 , 7 - 4 ) w5 ~ 1-i - (3<Ti+a; 3)ri 8 K - 1 ) 3 0 a 3 e t - ( 3 ^ „ + 3 e ) where Ee' 6 = D + »'£. Remark We have used o\ to transform the nonautonomous equation (7.8.1) to an autonomous one. We could have avoided using o\ by looking for a solution for B0 at the frequency 3(o"i + u;3/3) instead of a steady state solution of the resulting Chapter 7: Multiple Scales Solution • autonomous equation. This approach is taken merely for convenience. 114 With this notation, (7.8.1) becomes in real form (7.8.3) and (7.8.4) dip0 2 E3 3 <^ o&o^ — = -oiu0b0 - — 7 T ^ a o c o s ( ^ o + 30 - V>o) db0 1 w0^— = -u0gb0 - 7 + 1 E3 8 K - 1 ) 3 '8(u;o-l) 3 3 3 .3 , 6E2u0alb0 8W°b° + 8 ( W g - l ) 2 aosin(3^0 + 30 - ip0). We can get a more compact representation by putting Ea0 a2 - -2cj0Oi/g so we get instead r = b0/CYo xb0 = tl)0- 30 — 1 — 2a\ ( possibly negative) (7.8.3) (7.8.4) ' dr ch 37 a 2 r - - a 3 cos(^ 0) r(R20-r2)-^a3sm^0) Chapter 7: Multiple Scales Solution Thus, at steady state, by squaring and adding appropriately we get 115 (7.8.5) «y + r\Rl-r^ = \a\ This is a cubic equation for r 2 , which allows us to find the steady states for bo. Remark For a consistent asymptotic expansion, we note that o, D, and B are (at this moment unspecified) functions of u0. This means that for convenience and consistency we do not replace each occurrence of u0 in the above equation with 3, and likewise when the time comes to evaluate B, D, and g, we use the exact value of UJ0. This may seem unnecessary, as the computed value of 60 is accurate only to O(l), with errors O(fi), and wo = 3 + O(fx) here, but it is a valid procedure, and convenient for programming. For hand computation of a less complicated problem, it would make sense to evaluate the parameters at UJQ = 3 and use those values throughout. Here it is easier to make the parameters dependent on the wind speed, and any errors introduced will be of higher order. We can evaluate £ 3 = 3<p0 + 30 — ipo at steady state once b0 is known by using (7.8.3) and (7.8.4). This completes the solution to O(l) in the subharmonic reso-nance case. Notice that Ao is completely unaffected by the subharmonic resonance. Note that what is left in the Second 0(/x) equation is different than the solution Chapter 7: Multiple Scales Solution of (7.6.12), being 116 (7.8.6) d = P 1 ( T 1 , r 2 , r 3 ) e l ^ r + K l e i T + « 2 u ) 0 _ 1 e t ^ - 1 ) T + cc. where K2wit + 1 W 0 2 ^ - ^ ( (*I> - + g\ - Z~i\(2vv + A A ) - Z^v\A''eluJ=Ti 71/ 3 ^ - (3u;0)2 _ _ _ 3 T ^ 2 A _ _ - (2w0 + l ) 2 = 3 ^ 2 A 3 T f * A 2 _ , W 3 r i 2 w ° - 1 w g - ( 2 u / 0 - l ) 2 u 0 2-(u; 0 + 2 ) 2 e This should be compared with (7.6.13) to appreciate the differences. The component at frequency 1 has a new, apparently rj-varying term, the terms at frequencies w0-2 and 3 are absorbed, and the u0 + 2 and 2w0 — 1 frequency terms combine. The first 0(//3) equation in the subharmonic case differs from (7.7.1) in that there are some terms involving <7i, which was zero in the nonresonance case. We Chapter 7: Multiple Scales Solution have 117 (7.8.7) d2Yj dT2 dTdn , d2Y, _ 'dTdT2 dT2 d2Yx dTdrx 2^ d2Yi d2Yx d2Y0 d2Y0 dTdrz °ldTdrx d2Y0 dr2 - (2o3 + 2oxo2) dT2 - (4o2 + 2 C T 2 ) 2 d2Y0 ^ dTXdr2 dT2  d2Y0 dr2 dT dT d2Y0 dTdn dY0 6\dY, dT dT The anti-secularity equation is thus more complicated, being (7.8.8) - 2 ^ + 2 c r 1 ^ 2 = -e- t ( T^' dn fn(r 2,r3,r 4) where dA\ (7.8.9) fn(r 2, r 3 , r 4 ) = - 2 * - ^ + (2a 2 - 2CT2).41 OT2 .dAr> dAo , . , - 2i —- - 2ox-~- + 2tr3 - 2aia 2)^o + ^ r i ^ i - S r ^ 2 ^ + 2A0A~oM\ - 7r 7[15^^o^i + 20-4po^i] + s • KXe Chapter 7: Multiple Scales Solution 118 To avoid secularity in (7.8.8) on the ri-scale, we must have fn(r 2 ,TS ,T4 ) = 0. This gives, as before, (7.8.10) A2{T1,T2) = A2{r2)e-lff>T' Remark el<TiTi KX is in fact independent of r 1 ? as long as BQ is at a steady state. From (7.8.6) we have (7.8.11) /cx = • ( (iD-B)A1(r2,T3)e-™^ -D - i B , , i n T + g • —-2 7-Ao{T2,T3,T4)e-ia>T> w0 - 1 - 3 7 - ~ D 2 ~ \ B A0{T2,T3,T4)e-iaiT> [2|i/|2 + |A| LO0 - 1 - 37^0^50(7-!, 7 " 2 , 7"3, r 4)-and as w3 + 2<7i = —<7j by (7.8.2), we see that the only dependence on T\ is through BQ. Thus, if BQ is at a steady restate, this last term must be included in the above anti-secularity equation, to avoid ri-secularity in A\. This inclusion will affect the stability analysis later. When we convert (7.8.9) to real form we get, with raj, m 2 , and m3 as in (7.7.7), (7.7.8), and (7.7.9) respectively, and with the real form definitions as in the nonres-Chapter 7: Multiple Scales Solution onance case (e.g. Ax = ^aie1^1), 119 (7.8.12) _ S l _ = ( 0 l _ 0 ; _ . - ^ _ ^ . 1 d0 o d0 o , » , .+ a 0 — h oiao— 1- (a 3 - a2oi)a0\Cd OT3 OT2 da0 da0 - mi • ]-ai • s2d + rn2 • (-Ded + Bsd) + s • 0/ 2 ^ 3 sm(V>o - 30o - 20 + 4>d) where EelQ = D + iB as before, and the imaginary part becomes da\ d<Po °<po (7.8.13) — = \ao-^r + o-xdo-^- + (cr3 - 020i)ao\Sd da0 da0 . - ^ + °l~dV2]cd + mi • ]-ai • c2d + m 2 • {-Bed - Dsd) 1 + m3 • -ax — s 3^u0b0alE2 8 K - 1)3 cos(0o - 300 - 20 + <pd) The solution of these equations parallels the solution of (7.7.5) and (7.7.6) pre-cisely. We again simplify the solution by choosing cr3 so that sin(0d) = sd = 0. Also, to make the limit cycle solution actually a steady state, we choose as in the nonresonance case Chapter 7: Multiple Scales Solution 120 Thus at steady state we have (7.8.14) mi + m 3 2cd m2B + s • Y cos(^) where ^z = ipo — 3<f>o ~ 20 is known, as are the other quantities. Again, the choice 4>d = 0 or 7T is immaterial, as the sign cancels out as before. Also, we have <73 = nance case, it all goes through except for one point: the anti-secularity equation with which we do the stability analysis is only necessarily valid if Bo is at a T\-steady state. Given that restriction, we can say that a\ is stable if and only if the corresponding ao is stable. 7.9 Superharmonic Solution to 0(/z) Remark This section was included for completeness. When we calculate the superharmonic resonance for the case of oscillation in air, we find that the O(l) solution ao is zero in this region, and the maximum amplitude of the next term is less than 10 - 5, which is insignificant. For the case of water, for larger n, this term may be significant, however, and thus the solution is included here. The analysis of a2o-i + (m2D - s • 8 K 2 _ ; ' ) 3 sin(ed))/a0. Remark When we wish to use the same stability analysis as in the nonreso-Chapter 7: Multiple Scales Solution 121 this case is very similar to the analysis of the subharmonic case. The second 0(/x) anti-secularity equation is, taking w0 = 1/3 + fj-u>i/s, dB (7.9.1) -2iu0—^ + 2o^lB0 = -iuj0gB0 + 1 Zv2v + 6XXv + Su2Xe~l3uJi^n which leaves as the solution of the second O(p) equation (7.9.2) where C, = JB 1(r 1,7- 2,7- 3) C 1' W o T + « i c t ' ( 1 ) T + iC2 W o + i e ^ 2 w « + 1 ^ + K W o + 2 e i ( w o + 2 ) r + /c 3 e l ( 3 ) T + cc. K -1) [iD - B)Ai + gX - 7(i/3eI'-3w'/»Tl + A(6I/I7 + 3AA) ^2u>„ + 1 — - 3 7 + I u2-(2u0 + l)2 - 3 7 1 / A 2 l / 2 A + i72A2 e- t'-3^/=n K w o + 2 — / 2 « 3 UJ2 - (w0 + 2)2 - 7 A 3 W g - S 2 Now, equation (7.9.1) is ri-autonomous if and only if Ae ' ' 3 w i / 3 T l is independent of Chapter 7: Multiple Scales Solution 122 T\. This occurs if A0 = 0 (=• A = 0) or (7.9.3) ai = -3w 1 / 3 Not coincidentally, this choice of ox makes K\ and /C2w„ + i independent of TI also. Putting for convenience (almost as in the subharmonic case) r = b0/CYn = ^0 - 0/3 Eeie = D + iB <j>o = 0 Oil = £ a 0 Cy 0wo(wg - 1) Rl = \- 2a\ a2 = -2u>0oi/g r = -gri we have as the real form of the anti-secularity equations (7.9.4) r - f^ = a 2 r + air2cos(3r/)o) OT dr — = r{R2Q - r 2) + axr2 sin(30o) OT Chapter 7: Multiple Scales Solution 123 R e m a r k The range of values of a2 includes zero, when the wind speed is precisely 1/3. Note also that ax is zero when ao is zero. We investigate some special case solutions of (7.9.4), as a prelude. If ao = 0, the solution is particularly simple. In this case, c*i = 0 also, and thus the solution is (7.9.5) ^O = CC2T + P{T2,T3,T4) r = (l + K ( r 2 , r 3 , r 4 ) e - 2 ' ) - 1 / 2 or else the unstable solution r = 0. Note that this solution is not a steady solution unless c*2 = 0. This case will need careful analysis later. To find any steady-state solutions in the general case, we must solve the poly-nomial equation (7.9.6) r2ot2 + r 2 ( R 2 - r 2 ) 2 = a 2 r 4 which is easily seen to have solutions r = 0 (7.9.7) r 2 = R2 + \a\ ± yj'R2a\ + a\/A - a2 Note that unless a2 > | , R2 > 0. We can easily see that if a2 < {R2 + a 2 /4)a 2 Chapter 7: Multiple Scales Solution 124 then there will be three nonnegative steady states. The corresponding tpo will be given by setting the right hand sides of (7.9.4) to zero. For each nonzero r, we will get 3 solutions for xpo- This will give 6 steady states in all. If the above inequality for a 2 is violated, that is if the wind speed is too far from the exact superharmonic resonance, there are no steady-state solutions. A final special case to consider is what happens exactly at the resonance, when o\ = 0. The above inequality is satisfied for all ay, and our steady states become (7.9.8) r = \ax + yj R* + aj/4 2 7T 57T 37T 6'T'Y and (7.9.9) r = -\ax + y/R* + a\J4 r- W 7n HIT 2'~6"'~6~ and a simple stability analysis shows that the eigenvalues of the Jacobian are —3r2 + 2ai sin(30o)r + RQ and — 3aj sin(30o)- Thus, since ay < 0, the steady states are unstable if 4>o = 7r /6 , . . . and can only be stable if rjj0 = 7r/2, We may now find the steady-state value of the O(fi) term for Y. The anti-secularity Chapter 7: Multiple Scales Solution 125 equation for the first 0((xz) is d A (7.9.10) 2t—- - 2oyA2 = e'iaiTl fn(r 2,r 3,r 4) + term where fn(7-2,7-3, r4) is different, and 'term' may or may not be present, depending on whether Bo is at a ri-limit cycle or at a Tj-steady state. If Bo is at a ri-steady state, then 2> t n - d A \ (7.9.11) fn{rj,T2,T3) = 2(a2 - of)Ay - 2i 2 B - 57-2 -7A1 + 2(cr3 - oxo2)Ao + tl ( f ! + a j A t - %rz\A%Ax + 2A0A0A1] + + 5r 5 [ 4 i 4 0 ^ 0 ^ i + GAl~A20Ai} - 7 ^ ( 1 5^0^! + 20A^ 0 ^!] + *( i - 7(3AA + 6i/Z7)] 71/3 — s-K - 1 ) If, however, Ao is zero, then Bo is not at a steady state but rather at a limit cycle. In this case, the term i / 3 e*- 3 w i /3 r ' = const . e*'-(3»i"'«+3wi /3) T i = const . e ^ a i + S M^/c - i ) ^ = const •e i' 3 u ; i/ 3 < T , T 2 Chapter 7: Multiple Scales Solution 126 and the only way that this can be equal to e~tCTlTl is for Wx/3 = 0. Thus, when w i / 3 7^ 0? the extra term goes into the ri-equation for A2, and not into the r 2 -equation for Ai. In addition, the T 2 equation for A\ is much simplified, having as solutions functions of r 2 which decay exponentially to zero, as long as the zero solution for AQ is stable in the 0(1) sense. Also in this case, the equation for A2 is linear and easily solved. However, if — 0, then for any choice of oj the u3 term must be included in the equation for A\, in which case the analysis proceeds as before, except for some more 72-modulation of the phase. Solutions: Case I, AQ ^  0 The anti-secularity equations in real form are dfid 2 B \ (7.9.12) a x - — = (a 2 - tTj - s--^ -r ) a x + p i c d dr2 2(LO^ - lj - mxaxSrfCd + m2Bsd da,\ 2 (7.9.13) = pisd + mxajc^ - m2Bcd or2 where mx, m2, and m 3 are as in (7.7.7)—(7.7.9), so as before m\ = m 3 = /'(ao) whenever /(ao) =0. Also, (7.9.14) m 4 - S l u 2 ° b * 8 K -1) Pi = {o~3 - Oia2)a0 - m2D - m 4 sin(30o) Chapter 7: Multiple Scales Solution 127 B We choose as before o2 = o\ + s2(J*-\\ s o w e n a v e a ^ steady-state Pi - st + cd(mxaicd - m2B) = 0 Pi • cd - sd(miaicd - m2B) = 0 Thus, multiplying the first by sd = sm(<j>d) and the second by cd and adding, we get pi (sd + cd) = 0, and thus pi = 0. Since in this case ao 7^  0, we use the only unknown present in pi to get a3 = o2Oi + — ( m2D + m 4 sin(30o) Then, similarly, (sd + cd)(miaicd — m2B) = 0 and thus ^ rn2B (7.9.15 a l C d = — L -mi as in (7.7.12). Remark This is precisely the same form as in the nonresonance case. How-ever, note that 60 and hence m2 is determined by a different equation than in the nonresonance case, so that we may expect numerical differences. Case II: ao = 0 In this case, BQ is at a limit cycle rather than a steady-state, and this changes Chapter 7: Multiple Scales Solution 128 the analysis. At the limit cycle, we have bo = cy n thus the anti-secularity equation for the first 0(fx3) equation is - 2 i ^ + 2oXA2 + is •T°C\ • c«((3«i/3-3W„^)r.+3^) (2(a2 - °" - s2^h))A> - 2idt2 + WW**) =° Note (and this is crucial) that the T\ frequency of the 5 7 term is not equal to o\ — 3^/3 unless W1/3 = 0. In fact we will see that if u>i/3 = O(fi) then we are in a different subcase. Case Ila: u^/3 ^  O(n) We must, as before, have the coefficient of e _ l < T l T l = 0. This gives dAx dr2 which implies A^K(r2,r3,T4)ef'^ which for any fixed values of r 2, r 3, and r4 tends to zero exponentially if and only if the zero root is stable (recall the zero root is stable precisely when /'(0) < 0). The Chapter 7: Multiple Scales Solution 129 other equation, lor A2, is linear and easy to solve. Putting ra5 = \rne we get A2 = A'2 (r2, r 3 , r4)e—' + i ^ e ^ ' *« which is 0 ( 1 ) unless o\ = 0(£t) which occurs precisely when W\/z = O(A0- Thus we see that the superharmonic resonance has a special effect in a nearer neighborhood of u;0 = 1 /3 . Case l i b : u0 = 1/3 + fJ-2u\/z Notice the change in the meaning of the symbol W j / 3 . This should not cause con-fusion, as this usage will be confined to this section. Notice also that here o~\ = 0, and so ipo — 4>o{T2iTz-,r4)-, but as before b0 = Cyir In this case the anti-secularity equation for the first 0(n3) equation is .dA2 .dA\ . 71/3 , 0 , , OTI dr2 [w* - 1) Thus to avoid secularity we must have = 0 and to solve the remaining equation we must know the dependence of ipo on r2. The second 0(n2) equation, in this special case, is very simple: dr 2 2(u)^ - 1) 1 dB\ . _, Chapter 7: Multiple Scales Solution 130 - 3 1 7 ^ 5 ^ ! - isu0/ 2 B ,-Bo J = 0 K - 1 ) ) and as usual we set the brackets to zero separately, and this gives dB0 B "5 lsT~2 7Two-Bo = 0 dr2 (wg - 1) so ipo(r2, T3, T4) = 2a2u>oT2 + ipo{T3,u)- This means that Ax = A \ e f ' ^ + m 6 C * ( 3 w . / 3 ^ + 3 ^ ( ^ . - . . ) ) where j4cYn m < 3 tS16(u;2 - l)[-/'(0) + t(3w 1 / 3 + 6tr2u;o)] and we need only calculate the magnitude of this to find the amplitude. Note that the A\ term is immaterial, as it decays exponentially to zero. Conclusion This completes the solution of the model equations to 0{n) in Y and 0(1) for Cv. 7.10 Results of the Method Of Multiple Scales What follows are some graphs of the solutions to O(fi) of the model equations. We give the root mean square amplitudes as a means of comparing with the data from [l]. In each graph, the amplitudes are those of the solutions to O(n), so Chapter 7: Multiple Scales Solution 131 Yo + and Co + nC\ are each represented. The parameters used are those fixed by experiment, with reasonable values for the parameters outside the resonance region. We have 9 graphs of the results of the multiple-scales solution. Figures 7 . 1 0 . 1 through 7 . 1 0 . 6 compare the data from the low turbulence, medium turbulence, and high turbulence level experiments of [l], alternating amplitude of oscillation in the odd figures with the amplitude of the wake oscillator in the even figures. Figure 7 . 1 0 . 7 is an ad hoc parameter fit showing the ability of the model to exhibit significant subharmohic resonance. Figures 7 .10.8 and 7 . 1 0 . 9 show the predictions of this method of solution for the case of larger n occurring in the hydrodynamic case, cf [5]. We examine first Figures 7 . 1 0 . 1 to 7 . 1 0 . 6 , the aerodynamic case. We see that the agreement is reasonable, even in the low-damping, low-turbulence case, presented in Figures 7 . 1 0 . 1 and 7 . 1 0 . 2 , where the interaction of the galloping and the vortex-induced oscillation is the greatest. The model correctly predicts the onset of the nonzero amplitude of oscillation in all cases, and correctly predicts the growth of the amplitude of oscillation. A noticeable feature is the 'overshoot' occurring near the end of the resonance region. As the O(n) solution in the resonance region does not depend on the quasi-steady parameters Ak or the damping this solution is the same for all cases with the same turbulence level. When we look at the 0 ( M 2 ) Chapter 7: Multiple Scales Solution 132 solution, hoping for more accuracy, we see that the solution begins to oscillate near UIQ = 1.04 (cf Figure 7.5.1), while the 0(u.) solution appears to behave in the manner expected; that is, to grow large and meet the nonresonance solution which is becoming small at this point. This is a graphic demonstration of the power of this asymptotic method, as the one term solution can not be expected to be accurate, but turns out to be so anyway. When the two solutions, the O(p) and the 0(/x2), agree reasonably, we can be sure that the error made by the 0(/u) solution is less than the difference between the two. However, when the difference is large, as it is in the resonance region just after UQ = 1.04, this error estimate does not help. In fact, we can reasonably expect more accuracy than is indicated, so it is likely that the O(p) solution is as accurate as it needs to be. The fact that the two regions match up reasonably well in spite of the fact that the error is predicted to be large gives confidence in the solution at this point. Notice also a kink in the O(p) solution at the left end of the nonresonance range, particularly in the higher-turbulence figures in Figure 7.10.3 and 7.10.5. This, too, is spurious, and is caused by the asymptotic solution trying to match the behaviour in a different range. In this case, however, it is the O(fi) solution indicating that the error made by the O(l) solution may be becoming large. However, for this aerodynamic case, we see by comparison with Figure 5.3.1, the solution by the method of Van der Pol, that the errors made are in fact quite small. Chapter 7: Multiple Scales Solution 133 In Figure 7.10.2 we see the predicted RMS excitation compared with the data taken from [l]. The agreement is reasonable, reflecting the general trend of the data, and indicating a peak near the resonance region. However, the low damping data shows a clear decreasing trend, which is not reflected in the predicted solution. This is caused by choosing Cy 0 as a constant from the fixed-cylinder experiments. It is interesting to note that a clear decreasing trend was observed in some cases in experiments by the authors of [l] prior to those reported in [l], but the amount of the decrease was not considered significant. In Figures 7.10.4 and 7.10.6 the accuracy is noticeably better, in spite of the fact that the corresponding solutions for the medium and high damping cases in Figures 7.10.3 and 7.10.5 are worse fits than in Figure 7.10.1. This is not surprising, because for the higher-damping cases the wake vortex system is not as important for the amplitude of oscillation as the shear-layer instability. The poor fit of the higher-damping amplitudes of oscillation is probably due to the poor fit of the cubic polynomial used to approximate the lift coefficient data. This observation is borne out by noticing that the low damping cases are well predicted for all turbulence levels, due to the better fit of the polynomial to the data. For the functional form of the parameters used in Figures 7.10.1—7.10.6, that is, a(u0) = aw0, D[wo) = D/u0, and B(u0) = B/UQ, we get good overall quantitative agreement, but the kink associated with the subharmonic resonance is not present. Chapter 7: Multiple Scales Solution 134 If instead we choose a(u>o) = 0.50U;Q, B(WO) — -5.29 + 2.94W2,, then in the low damping low turbulence case, we get a kink near LUQ = 3 that is very much like the one observed (Figure 7.10.7). This parameter fitting is rather ad hoc, but does not conflict with any of the parameter fixing done earlier, as the parameter fitting is done in the resonance region. As u>o gets larger, though, we expect more unrealistic behaviour, as the parameter a(uo) can no longer be considered small. A more serious problem with the model in general is the location of the sub-harmonic resonance, observed physically in [l] to be near cvo = 2.5, significantly different than the u>o = 3 predicted here. This prediction is inherent in the model equations, and is not an artifact of the method of solution. One possible physical correction to this would be to have the Strouhal number shift to account for the change, so that LO0 = 3 = U/Ur = 2nSU would occur in the correct wind speed region. This would require a 20% change in the Strouhal number, however, and this seems unrealistic. Figures 7.10.8 and 7.10.9 show the effects of larger n. As our solution is in the form of an asymptotic series in powers of the square root of n, the accuracy of our results is expected to be better as n —» 0, and thus we expect poorer solutions for larger n. The solutions presented here are however not too bad, outside of the large spikes in the resonance region. Comparison with the numerical solution of Bouclin [5] shows quite good agreement, after the resonance region. Bouclin's results for this Chapter 7: Multiple Scales Solution 135 set of parameters is contained in his Figure 23. Some data taken from that figure, corrected for RMS values, are plotted on Figure 7.10.8. The largest difference, of course, occurs in the resonance region. Before the resonance region, however, the difference is low in an absolute sense, but high in a relative sense, being about 50%. After the resonance region, at u>o = 1.2, the relative difference is only 8%, while at the extreme end of the range of Bouclin's figure, uo = 1.3, the relative difference is down to 4%. This suggests that the multiple scales solution will become still more accurate as we move away from the resonance region. Figure 7.10.9 shows the amplitude of excitation for the same parameters as Figure 7.10.8. Unfortunately Bouclin did not provide a numerical solution for the excitation, so we cannot compare. However, on comparing it to Figure 7.10.8 itself, we see that the amplitude of excitation is predicted to be large even after u>o = 1-2, where the difference between Bouclin's numerical solution and the solution by the method of multiple scales is less than 8%. This gives us some confidence that the amplitude of excitation is also correctly predicted in this region. However, it is obvious that the numerical solution of the model equations is feasible for this n, which is about 20 times larger than the n used in the aerodynamic case. Thus, though the method of multiple scales gives acceptable answers even in this case, at much less computing cost, the accuracy of the numerical method makes it possibly more preferable in this case, and probably more so for still larger n. However, for Chapter 7: Multiple Scales Solution 136 smaller n the computing cost of the numerical solution increases, while the accuracy of the solution by the method of multiple scales increases with the cost of solution remaining the same. Thus it is clear that there is some value of n above which it is better to use the numerical method, and below which it is preferable to use the asymptotic method. The precise determination of this value of n is of course impossible in this general context, depending as it does on the changing value of computing time versus the need for accuracy. However, with that caveat in mind, it is the belief of the author that the numerical method is preferable only when n = O(0.1) or larger, and that for smaller n the method of multiple scales will provide cheaper results with adequate accuracy. Chapter 7: Multiple Scales Solution 137 Figure 7.10.1 RMS Amplitude of Oscillation: Low Turbulence Case. O P = 0.00088 V P = 0.00298 A P = 0.00545 Chapter 7: Multiple Scales Solution 138 2-i 1.8 H 1.6H 1.4 H 1.2 0.8 0.6 H 0.4 H 0.2H of A A o c> 7 V A A A A A o - $ v Q D o n = 4.7x10~* a = 0 . 1 3 X U Q 1 0 = 0.855/w0 B = - 2 . 3 5 / « Q 2 C v = 1.40 *0 * 1 = 4.87 A 3 = 4.21x102 A , = 1.70x104 A? = 1.94x10 - i | A A A | A A A A A A i 1 4 5 6 7 8 9 CO 0 Figure 7.10.2 RMS Amplitude of Excitation: Low Turbulence Case. O 0 = 0.00088 V 0 = 0.00298 A 0.00545 Chapter 7: Multiple Scales Solution 139 1-1 0.9-0.8-0.7-0.6->- 0.5-0.4 0.3-0.2 0.1-n = 4.7x10 a = 0 . 1 3 X U Q 1 D = 0.855/&>0 B = - 2 . 3 5 / W 0 2 C v =1.40 T 0 A. = 3.95 A j = 5.14x10 A 5 = 0 A ? = 0 O A O \7 A O A A A A 0 1 AVA A A A A A A A / A | A A i r 2 3 4 5 6 7 8 CO 0 9 Figure 7.10.3 RMS Amplitude of Oscillation: Medium Turbulence O & = 0.00105 V P = 0.00296 A 0 = 0.00550 Chapter 7: Multiple Scales Solution 140 1.8 H 1.6 H 1.4 H 1.2 H H 0.8 0.6 H 0.4 H 0.2 - 4 n = 4.7x10 a = 0 . 1 3 X U Q 1 D = 0.855/CJ 0 B = -2 .35 /W Q 2 C Y = 1.40 A 1 = 3.95 A 3 = 5.14X101 A 5 = 0 A 7 = 0 b A 0 " # A A A A A A A ^ A A A A A 3 4 5 6 9 Figure 7.10.4 RMS Amplitude of Excitation: Medium Turbulence o 0 = 0.00105 V 0 = 0.00296 Case. A 0 = 0.00550 Chapter 7: Multiple Scales Solution 141 1n 0.9-0.8 0.7-0.6->- 0.5-0.4-0.3-0.2-0.1-n = 4.7x10~4 a = 0 . 1 3 X M Q 1 D = 0.855/u 0 B = - 2 . 3 5 / W 0 2 C v = 1.40 T 0 A = 3.15 1 A j = 4.71x10 A =0 5 A = 0 7 o V / / o / / o / / o o \7 V A A A A A ^ A 4 T" 5 A A ~r 8 CO 0 ~ i 9 Figure 7.10.5 RMS Amplitude of Oscillation: High Turbulence Case. o 0 = 0.00117 V P = 0.00295 A 0 = 0.00550 Chapter 7: Multiple Scales Solution 142 1.8 H 1.6 H 1.4 H 1.2 H H 0.8H 0.6H 0.4 H 0.2 H - 4 A n = 4.7x10 a - 0.13xu0 D = 0.855/OJQ B = -2.35/W-C Y = 1.40 T 0 A t = 3.15 A 3 = 4.71x101 A 5 = 0 A 7 = 0 A "A""" A A V ' AA W A A A A 1 1 1 1 1 1 1 1 1 0 1 2 3 4 5 6 7 8 9 Figure 7.10.6 RMS Amplitude of Excitation: High Turbulence Case. O 0 = 0.00117 V 0 = 0.00295 A 0 = 0.00550 Chapter 7: Multiple Scales Solution 143 0.8-0.7-0.6->- 0.5-0.4 0.3-0.2-0.1-n = 4.7x10 B = 8.8x10 -4 / a = 0.50x«Q D = 0.855/w0 B = -5.29 + 2.94xW( C Y = 1.40 T0 A = 4.87 2 A = 4.41x10 5 4 A c = 1.70x10 5 5 A, = 1.94x10 / .Si/ ' ?Ti / / / / / If Legend Stab I e_Pre - Sup er h ar m o ni c Stable Superharmonic Stable Pre-Resonance Stable_ Resonance Stable Post-Resonance Stable Subharmonic Stable PosJ-jSubharmonic y BGMP Experimental Data £5 r^-0 0.5 1 —I 1 1 1 1 1 1 1 1.5 2 2.5 3 3.5 4 4.5 5 Figure 7.10.7 RMS Amplitude of Oscillation Showing Subharmonic Resonance. /? = 0.00088. Chapter 7: Multiple Scales Solution 144 0.6-1 0.5-0.4->- 0.3-n » 7 . S 2 x W fi s *.4x10~5 a - 0 . 0 2 4 9 D = 0 . 6 0 B =-1.64 C v = 0 . 7 0 T 0 A f «= 2 . 6 9 A j = 1.69xK> 2 A g = 6.27X103 A ? = 5.99x104 0.2-0.1-0.0 9 Multiple Scales Solution (0 Bouclin's Numerical Solution [5] T 1 1 1 1 1 T ^ n 1—""I 1 T 0 0.2 0.4 0.6 0.8 1 1.2 1.4 1.6 1.8 2 2.2 2.4 CJ. Figure 7.10.8 RMS Amplitude of Oscillation: Hydrodynamic Case. Chapter 7: Multiple Scales Solution 145 2-1 ; n = 7.32x10"3 p - 4.4x10~5 1.8- '; a = 0.0249 D = 0.60 B =-1.64 1.6-1.4-! C v = 0.70 A 1 = 2.69 A = 1.69x102 s 3 A 5 = 6.27x10 A y = 5.99x104 1.2- i \ \ \ \ r 0.8- \ \ V 0.6- J \ 0 . 4 -0.2-| ! i ! n 1 0 I l D 0.2 l I l 0.4 0.6 0.8 1 1 1 1 1.2 1.4 CO 0 I 1 1 1 1 1.6 1.8 2 2.2 2.4 Figure 7.10.9 RMS Amplitude of Excitation: Hydrodynamic Case. Chapter 8 Comparison of Solutions With Each Other and With Experiment Not meaning to strike, but first—having summoned us together here, in this outest corner of the realm—to choose out, snap in two, throw on the midden, any blades of meaner mettle. —E. R. Eddison 8.1 Concordiat of Solutions We wish to compare and contrast the results of the various methods of solution, to decide which (if any) is the best for our purposes. This will serve the purpose of error-checking as well as providing some useful details of the solutions. One of the most useful features of the solutions is the prediction of the wind speeds at which non-zero amplitudes of oscillation are initiated, henceforth denoted by Ui or u, = Ui/Ur. We compare the results of the three methods; (I) The method of Van Der Pol, (II) Hopf Bifurcation Theory, and (III) the Method of Multiple Scales. For (I), the equations determining Y, Cv, and H, (5.1.5)—(5.1.7) are satisfied identically 146 Chapter 8: Comparison with Data 147 when Y = 0. We must instead look at the limiting case when Y jCv —> 0. After doing the analysis, we arrive at the following polynomial equation Pi (too) in the wind speed wo, in the case a(w0) = OJW0, B and D are constant, and where Wo = Uo/Ur is the onset velocity predicted by the quasi-steady theory: (8.1.1) P/(w0) = - Wo^t -{2-D-n- a 2)w 3 - W0{a2 - 2)w2 + (1 - Drj - aBn)u0 - WQ = 0 where n — Ur/A\. The roots of this quintic equation in wo are easy to find numer-ically, but we can investigate them analytically in the case a is small. First, however, we look at the determining equations from the other regions. From the Bifurcation theory, we get the location of the Hopf Bifurcation Points directly: 5 (8.1.2) Pu = PBM = ^2ciUl0 i = 0 where the c; are given in section 6.8. Closer inspection of these coefficients reveals that PuM = aPr{iOo) + 0{n) so we see that the roots of the first will, if n is small enough, be close to the roots of the second. This shows that the initiation points predicted by the method of Van Der Pol are within 0(n) (except of course for multiple roots, or near-multiple roots) Chapter 8: Comparison with Data 148 of those predicted by the simpler bifurcation theory, which is interesting, as the bifurcations are those from the zero steady-state, and the Van Der Pol predictions include those from the non-zero time-dependent solution with Cv 7^ 0. I believe that this is a result of some interaction between the two, but it is certainly not predicted by the bifurcation theory, and must be here regarded as a coincidence. Lastly, we look at the results of the Method of Multiple Scales. We must look at two different regions here, the resonance region and the nonresonance region (considering the first order analysis only). In the resonance region, ao = 0 always, so we must look at when the next order term is zero. Now, ax = 0 if and only if D cos £ 1 + , , , \ = 0 o(o0/tti) which occurs only if Dcos f < 0, and thus only on the f = 7r branch of the solution. In the cases that have been presented, in Figure 7.5.1 and later figures in Chapter 7, this branch has always been the unstable branch. It is not known if there are parameter values for which this branch is stable. This equation is independent of the damping /? and the quasi-steady coefficients Ak, and so any initiation points arising from this equation will be constant for all values of Wo = Uo/Ur. The above equation gives Bg DU2 OH — — _ -| 2D 2g Chapter 8: Comparison with Data or 149 (8.1.3) Ba nDU2 . In the nonresonance case, ao = 0 if and only if P i n = (u2 - l)(w 0 - W0) + w 2 ( ^ ) = 0 l This is a cubic equation in IOQ, unlike Pn(tOo) and P/(u>o), which are quintic. How-ever, we solve the polynomial for the root near 1 in the case a <C 1, and we see that the roots of all three are very similar. Expanding the root near 1 of Pii(too), we have Ba 2 f -1 to0 = 1 + h a — — 0 2D \ 2Dn (8.1.4) + 0(a 3 ) + 0(n) B (8(1 - W0) + 6Dn) - ^ + 1 - W 0 8D2 2D and of course the root near 1 of Pi (too) has the same expansion to this order. We compare this to the result from the method of multiple scales. Equation (8.1.4), in the case n = 5 x 1 0 - 4 , B = -2.35, D = 0.855, Ai = 4.87, and U0 = 0.75, gives too = 1 - 1.374a - 8.637a2 + 0(a 3 ) + 0(n) and (8.1.3) gives 2.138 x 10~4 , . to0 = 1 - 1.374a + : + 0(n) a Chapter 8: Comparison with Data 150 which, for a = 0.13, is a difference of —0.146, which is significant. If we choose a = O(yjn) as n —• 0, then equation (8.1.3) and equation (8.1.4) are not asymptotic to each other; they have a common limit, 1, as n —-> 0, and a common dependence on a, but the detailed behaviour is different. In Figure 8.1.1, we compare the location of the initiation points for the method of multiple scales with the location of the Hopf Bifurcation points (cf Figures 6.9.1 and 6.9.2). We see general agreement, but the initiation points predicted by the method of multiple scales seem more realistic, as they predict initiation of non-zero amplitude in the resonance region for all values of W0, while after W0 = 3.6 the Hopf Bifurcation Points disappear. This is because of the more general nature of the initiation points calculated by the method of multiple scales. Both methods do predict the occurrence of an initiation point near u0 = W0 for W0 > 2.5, which is in accord with experimental observations. Chapter 8: Comparison with Data 151 5-| LJ / U 0/ r Figure 8.1.1 Graph of £/, vs U0 for fixed n. 8.2 Behaviour in the Quasi-Steady Limit Next, we look at the roots of the polynomials P](UQ) and PJU(LL>O) as U0 oo. Chapter 8: Comparison with Data 152 In this case we assume D(UJO) = D/uo, so we get from PJ(UJQ) w D r ] Dn(Dr) + l) - an(B + aD) n,w_5. uo = Wo-w0 w$ + °{w° } while from Pm(uio) we get Of course, the quasi-steady theory predicts an initiation point of LJQ = WQ = Uo/Ur always, so it is good to see that this model agrees with the quasi-steady theory in the limit. It is interesting to note that if D(UJO) is taken to be constant instead of depending inversely on W Q , the asymptotic results above come out as u0 = W0 - Dr) + O(l/W0) as W0 -> oo which is still in agreement with the quasi-steady theory, but the error is much larger, and in fact would be noticeable at moderate values of UQ. Instead we note that for Uo/Ur > 2 approximately that we have good results from the quasi-steady theory. This supports the functional form D/UJ0 for D(u>o)-8.3 Comparison of Predictions In this section we discuss the varying predictions of the different methods of solution of the model equations, as presented in Figure 5.3.1, Figures 6.9.3—6.9.5, Chapter 8: Comparison with Data 153 and Figure 7.10.1. Each of these Figures uses the same parameter values, and should give similar results. It is easily seen that the solution by the method of Van Der Pol contains the stable solutions found by the method of multiple scales, by comparing Figure 5.3.1 with Figure 7.10.1. The agreement of the two methods is exact, as it should be, even at the end of the resonance region, where we expected trouble with the method of multiple scales. The extraneous branches present in Figure 5.3.1, commented on previously, are seen by comparison to the stable solutions in Figure 7.10.1 to be unstable. However, the bifurcation solutions presented in Figures 6.9.3—6.9.5 do not agree with the stable solution by multiple scales, at least for the low damping case. For the medium and high damping cases, the agreement is quite good between the methods, as far as the bifurcation solution goes. It is interesting to note that the solution by the method of Van Der Pol agrees with the bifurcation solution even in the low damping case, as the bifurcation solution shows an unstable solution arising before the resonance region, which matches exactly the initiation present in the solution by the method of Van Der Pol. The unstable branch of the solution by multiple scales is not presented here, but it has the same qualitative behaviour without matching the initiation point precisely. In fact, the difference between the initiation points predicted is —0.146, as calculated in the previous section. To sum up, the methods presented all have their strong points. The method of Chapter 8: Comparison with Data 154 Van Der Pol is simple and accurate whenever the solution is in fact of the assumed form; the bifurcation method is guaranteed accurate in the neighborhood of the Hopf bifurcation points; and the method of multiple scales gives an automatic stability and error analysis, gives the form of the solution as well as the numerical coefficients, and is efficiently programmed on a computer. On the disadvantage side, the method of Van Der Pol does not provide an automatic stability analysis. A stability analysis can be done, but amounts to solving a non-autonomous linear system of differential equations, which in general is harder than using the method of multiple scales on the original problem. Also, in the case where the assumed form of the solution is inappropriate, the method of Van Der Pol is inaccurate; further, no error estimate is available. The bifurcation method is a local method only, and for our model predicts only unstable solutions. An error estimate is available, but is useful only near the Hopf bifurcation point, and near the zero solution. The method of multiple scales appears to be the method of choice. It is perhaps less accurate than the method of Van Der Pol for this problem in the resonance region, because in that region the form for the solution is simple and well defined, which means that the assumptions of the method are satisfied. However, comparison with the solution by the method of Van Der Pol show that the multiple scales solution, even in the resonance region, is of adequate accuracy. Also, multiple Chapter 8: Comparison with Data 155 scales seems to be the only method to detect a subharmonic resonance. The extra complication of the solution is made up for by the wealth of information about the solution that is readily available. Chapter 9 Conclusions But even next morning, I woke to a dis-comfortable and teasing certainty that there was much forgot... —E. R. Eddison 9.1 Conclusions After examining the results of the various methods of solution of the model equations we arrive at the following conclusions: 1. The solutions of the model equations realistically model the combined effects of galloping and vortex-induced vibration. The solution behaves correctly in the limit as Z70 ^> UR, collapsing onto the quasi-steady solution, plus a Hartlen-Currie type solution in the resonance region. In the case UQ « UR, the solutions match the experimental data reasonably well. In the case UQ < UR, the solution correctly exhibits a stable zero solution for U < UR, and then becomes large when U ~ UR. The solution exhibits a noticeable subharmonic resonance for 156 Chapter 9: Comparison with Data 157 some values of the parameters, which seems to correspond with that observed experimentally in [1]. 2. The approximate analytical solution provided by the Method of Multiple scales gives a useful solution already at the O(l) level, although the O(n) terms are necessary for the resonance region and the subharmonic resonance region. The method successfully determines the stability of the model solution in a simple fashion. To O(p) = O(yjn) = O(OJ), the approximate solution predicts a super-harmonic resonance near UQ = 1/3 and a subharmonic resonance at LJQ = 3. 3. The solution by the method of Van Der Pol is less useful than the solution by the method of multiple scales, because although somewhat simpler, it does not provide enough information to be valid over a large enough range, and provides neither a stability analysis nor an error estimate. 4. The solution by the Hopf Bifurcation theory, while providing a useful 'quick and dirty' solution of the model equations does not provide enough information, as it predicts only unstable solutions, and these valid only in a limited range. Further, they agree with the data only by coincidence. To be useful, one would have to look at the bifurcation of solutions from the non-steady solution given by Cv = Cvcos(fit), Y = O(n). 5. The functional form of the free parameters needs to be determined more com-pletely by physical considerations for this method to be a true semi-empirical Chapter 9: Comparison with Data 158 approach, rather than fully empirical. 6. The amplitude of the solution outside the resonance region, to O(l), is deter-mined by the quasi-steady coefficients Ak and the coupling coefficient D. The coupling coefficient B makes a difference in the phase difference between the displacement and the excitation only, and the coefficient c(wo) affects only the time taken to get to a limit cycle. 7. The size of the subharmonic resonance region depends on the coefficient a(cj0), the coefficient B, and the coefficient D, as well as the quasi-steady coefficients. Further, the effect of the subharmonic resonance is O(n) on the amplitude of oscillation of the body, but is 0(1) on the amplitude of the wake excitation term. 8. For the case of aeroelasticity, the superharmonic resonance effects are very small. The subharmonic resonance region is much more important. 9. The method of multiple scales is not as applicable to the hydrodynamic case as it is to the aerodynamic case. In the hydrodynamic case, the model equations are as valid, but in the case of large enough n, the method of multiple scales becomes less accurate and the direct numerical solution of the mode] equations becomes more efficient. Thus we see that there is a value of n above which numerical solution techniques are more applicable to the equations in this case. The method of multiple scales is however adequately accurate for some regions Chapter 9: Comparison with Data 159 of the solution even in the hydrodynamic case, as shown by Figures 7.10.8 and 7.10.9. Note however that the value of n for which these were plotted is in the small end of the range of values occurring in the hydrodynamic case. 10. The fact that simply adding Cpy and Cv gives such good results has some im-plications for the physical model. It was mentioned in the first chapter that the quasi-steady model depends on the position of the time-averaged shear layers. The success of this model suggests that this concept makes sense even in the presence of a significant perturbation due to the wake vortex system. 9.2 Suggestions for Further Work For further investigation of the model equations, it seems necessary to 1. Experimentally determine the form of the free parameters a(ujn), B(u>o)-, and D(LOO). Several forms were tried here, with some success, but these need to be put on a firmer base. Forced vibration experiments along the line of [2,16] might provide the necessary information. Particular attention should be paid to the resonance region, but the subharmonic resonance region(s) should not be neglected. 2. Investigate the predictions of this model in a three-dimensional situation, using an analysis similar to that in Sullivan [24]. Sullivan reported some interesting interactions of galloping and vortex-induced oscillation in a three-dimensional Chapter 9: Comparison with Data 160 setting, and it would be useful to see if this model was capable of explaining this. 3. The location of the subharmonic resonance region in the solution was not ex-actly reproduced by the experimental data. The subharmonic resonance region appeared around the region u>o = 2.5, and not around LOO = 3. This may be explained by a nonconstant Strouhal number, but this is unrealistic. It would be interesting to see if a more appropriate self-starting oscillator could be found, that would model this more closely. The following suggests itself: Cv + u20Cv = a(Cv - ^C^C^12). These equations are more difficult to solve, but preliminary investigations sug-gest that this equation would exhibit a subharmonic resonance (i.e. terms of frequency near 3) when LOQ was near 2.5. 4. The presence of large amplitude 'spikes' in the resonance region is undesirable. It is possible that different time scales would give a better result in this region. In particular, the time scales T, T\, T2, and r3, where as before r, = n*T, but where now n3 = n instead of y2 = n. This makes for a little more work, but in the resonance region Yo is still 0, but with \i being larger there may be smaller problems with the transition zone. In addition, several interesting theoretical questions were brought up in the course of Chapter 9: Comparison with Data 161 this study. It would be interesting to investigate the connection between the steady-state Hopf Bifurcation points and the nearby non-steady bifurcation points, in order to explain the observed coincidences of predicted non-zero amplitudes of oscillation with the experimentally observed oscillation. If successful, such an analysis would have the advantage of being much more general than the current analysis using the method of multiple scales, inasmuch as more general nonlinearities would be included automatically. The use of the method of multiple scales presupposes that the actual solutions of the model equations are bounded. No proof of the boundedness of the solution in the present case was attempted, as it is irrelevant for the practical case under consideration; a simple redefinition of our model to be only the bounded solutions of the model equations is sufficient to justify the analysis. However, it would be intellectually satisfying to have such a proof; or, considering the large amplitudes predicted near the end of the resonance region by the method of multiple scales, a proof that under some circumstances that the solutions to the model equations were not bounded. Lastly, recent interest in this type of model has been expressed for cylinders of different cross section. It might be expected that this model will be directly applicable to a 'D'-section cylinder and to cylinders of rectangular cross section, merely by adjusting the quasi-steady parameters Ak, as the quasi-steady theory has Chapter 9: Comparison with Data 162 already been worked out for these (for references see [18]). However, the effect of the geometry on the other parameters a(w0), B, D, etcetera needs to be investigated and may throw some light on the physical significance of these parameters. Bibliography [l] P. W. Bearman, I. S. Gartshore, D. J. Maull, and G. V. Parkinson, "Experiments on Flow-Induced Vibration of a Square-Section Cylinder", Journal of Fluids and Structures 1, (1987) pp 19-34. [2] P. W. Bearman and E. D. Obasaju, "An experimental study of pressure fluctu-ations on fixed and oscillating square-section cylinders", J. Fluid Mech. (1982) vol. 119, pp 297-321. [3] C. M . Bender and S. A. Orzag, Advanced Mathematical Methods for Scientists and Engineers, McGraw-Hill (1978) QA371.B43 [4] R. D. Blevins, Flow Induced Vibration, Van Nostrand (1977) TA355.B52 [5] D. N. Bouclin, Hydroelastic Oscillations of Square Cylinders, M.ASc. Thesis, University of British Columbia (1977). [6] S-N. Chow and J. K. Hale, Methods of Bifurcation Theory, Springer-Verlag (1982) QA372.C544. [7] E. R. Eddison, The Zimiamvian Trilogy, Ballantine Books (1968). [8] C. C. Feng, The Measurement of Vortex Induced Effects in Flow Past Stationary and Oscillating Circular and D-section Cylinders, M.ASc. Thesis, University of British Columbia (1968). [9] J. K. Hale, Ordinary Differential Equations, Wiley-Interscience,21 (1980), QA372.H184. [10] R. T. Hartlen and I. G. Currie, "Lift Oscillator Model of Vortex-Induced Vi-bration", J. Eng. Mech. Div. Proc. Amer. Soc. of Civ. Eng., Oct 1970 p 577. [11] A. C. Hearn (Ed.), REDUCE User's Manual, Rand Publication CP78 (1984). 163 164 [12] G. Iooss and D. P. Joseph, Elementary Stability and Bifurcation Theory, Springer-Verlag (1980) QA372.I68. [13] J. Kevorkian and J. D. Cole, Perturbation Methods in Applied Mathematics, Springer-Verlag (1981) QA1.A647. [14] N. Minorsky, Nonlinear Oscillations, Van Nostrand (1962). [15] A. H. Nayfeh and D. T. Mook, Nonlinear Oscillations, Wiley-Interscience, (1981) QA402.N34. [16] E. D. Obasaju, "Forced-Vibration Study of the Aeroelastic Instability of a Square-Section Cylinder Near Vortex Resonance", J. Wind Engineering and Industrial Aerodynamics, 12 No. 3 Sept 1983 pp 313-327. [17] G. V. Parkinson, "Aeroelastic Galloping in One Degree of Freedom", Symposium on Wind Effects on Buildings and Structures, paper 23 (1965). [18] G. V. Parkinson, "Mathematical Models of Flow-Induced Vibrations of Bluff Bodies", Flow-Induced Structural Vibrations, Proc. IUTAM-IAHR Symposium, Karlsruhe, Springer-Veriag (1974). [19] G. V. Parkinson, "Hydroelastic Phenomena of Bodies of Bluff Section in Steady Flow", Separated Flow around Marine Structures, Proc. Int. Symposium, Trond-heim, (1985). [20] G. V. Parkinson and J. D. Smith, "The Square Prism as an Aeroelastic Non-Linear Oscillator", Quarterly Journal of Mechanics and Applied Mathematics, XVIII part 2, Clarendon 1964. [21] A. B. Poore and A. R. Al-Rawi, "Some Applicable Hopf Bifurcation Formulas and an Application in Wind Engineering", Bifurcation Theory and Applications in Scientific Disciplines, Annals of the New York Academy of Sciences, vol 316 (1979) pp 590-604. [22] A. B. Poore and A. R. Al-Rawi, "The Dynamical behaviour of the Hartlen-Currie Wake Oscillator Model", Proc. 5th Int. Conf. Wind Eng., J.E. Cermak, ed. Pergamon (1979) pp 1073-1083. 165 [23] J. J. Stoker, Nonlinear Vibrations in Mechanical and Electrical Systems, Inter-• science (1950) QA871.S778. [24] P. P. Sullivan, Aeroelastic Galloping of Tall Structures in Simulated Winds, M.ASc. Thesis, University of British Columbia (1977). [25] D. H. Turnbull and I. G. Currie, "Flow-Induced Oscillation of Cylinders in the Streamwise Direction", Symposium on Flow-Induced Vibration 1, ASME (1984), pp 73-84. [26] M. A. Wawzonek, Aeroelastic Behavior of Square Section Prisms in Uniform Flow, M.ASc. Thesis, University of British Columbia (1979). [27] K. N. Wood, Coupled-Oscillator Models for Vortex-Induced Oscillation of a Cir-cular Cylinder, M.ASc. Thesis, University of British Columbia (1976). 


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