UBC Theses and Dissertations

UBC Theses Logo

UBC Theses and Dissertations

Anomalous commutators and the BJL limit Rogers, Duncan M. 1987

Your browser doesn't seem to have a PDF viewer, please download the PDF to view this item.

Item Metadata

Download

Media
831-UBC_1987_A6_7 R65.pdf [ 1.3MB ]
Metadata
JSON: 831-1.0085250.json
JSON-LD: 831-1.0085250-ld.json
RDF/XML (Pretty): 831-1.0085250-rdf.xml
RDF/JSON: 831-1.0085250-rdf.json
Turtle: 831-1.0085250-turtle.txt
N-Triples: 831-1.0085250-rdf-ntriples.txt
Original Record: 831-1.0085250-source.json
Full Text
831-1.0085250-fulltext.txt
Citation
831-1.0085250.ris

Full Text

A N O M A L O U S C O M M U T A T O R S A N D T H E B J L LIMIT by DUNCAN M. ROGERS B.Sc, York University, 1985 A THESIS SUBMITTED IN PARTIAL FULFILLMENT OF THE REQUIREMENTS FOR THE DEGREE OF MASTER OF SCIENCE in THE FACULTY OF GRADUATE STUDIES DEPARTMENT OF PHYSICS We accept this thesis as conforming to the required standard THE UNIVERSITY OF BRITISH COLUMBIA August 1987 ©Duncan M. Rogers, 1987 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 of Physi rs The University of British Columbia 1956 Main Mall Vancouver, Canada V6T 1Y3 Date Octofip.r 10, .1QR7 i i Abstract The BJL limit is derived and used to calculate the anomalous vector current com-mutator in QED. It is then shown, by a calculation with the BJL limit for double commutators, that the Jacobi identity fails for two vector currents and one axial vector current in QED. i i i Contents Abstract ii List of Figures iv Acknowledgement v 1. Introduction 1 2. Schwinger Terms and Seagulls 1 3. The Bjorken-Johnson-Low Limit 4 4. The Vector Current Commutator in Quantum Electrodynamics 5 5. The Bjorken-Johnson-Low Limit for Double Commutators 8 6. The Jacobi Identity Failure 9 7. Conclusion 13 References 14 iv List of Figures 1. One loop diagram for T*^ 7 2. One loop diagrams for T*^va 1 Q Acknowledgement I would like to thank Dr. Gordon W. Semenoff for helpful discussions. 1 1. Introduction Calculating current commutators in field theory is an ambiguous task. The problem of operator ordering in currents containing products of operators gives rise to infinities. It is not easy to define a method which takes an unequal time commutator into an equal time commutator. Fortunately, there exists a procedure which appears to overcome these difficulties. This method calculates the commutators from the well known Green's functions of field theory and lends itself well to perturbative techniques. The procedure is called the Bjorken-Johnson-Low (BJL) limit. But the results obtained with the BJL limit are often different from the values found using canonical commutation relations. Even worse, at times the Jacobi identity actually fails when calculated with the BJL limit. Before we discuss the BJL limit and the anomalies we should look at some results concerning time ordered products and equal time commutators. 2. Schwinger Terms and Seagulls The equal time commutator of operators A and B can be written as [A(t,x),B(t,y)] = C(t,x)63(x-y) + Sl(t, x) —- {63(x - y). dx1 The terms proportional to the derivative of the delta function do not arise from canon-ical commutation relations. They were first postulated by Schwinger1 for current-current commutators in electromagnetism and are called Schwinger terms. Higher order derivatives of the delta function may also be present. We write the time ordered product of A and B as T(x,y) = TA{x)B(y) = 0{xo - y0)A[x)B[y) + % 0 - x0)B{y)A[x). This is not in general Lorentz covariant. We therefore define the covariant time ordered product T*(x,y) by T*{x,y) = T{x,y) + T{x,y) 2 where r(x, y) is the covariantizing seagull. To find the explicit form of the seagull in terms of the Schwinger term we first introduce a unit timelike vector n** and the spacelike projection operator Then we write the noncovariant expressions in terms of n, \A{x),B(y)] 8({x - y) • n) = C(x; n)64(x - y) + S»P^—-6A(x - y) (1) OXis and T(x,y;n) = 9{{x - y) • n) A{x) B{y) + d((y - x) • n)B{y)A{x). The T* product is, of course, n independent, T* (x, y) = T(x, y; n) + r(x, y;n). We next vary T* with respect to n, remembering that only spacelike variations are permitted since n 2 is constrained to unity and n is timelike, G YXr G 7% = o. Using the commutator of equation (l), this becomes P ^ ~ r ( x , y ; n ) = P^S^x;n)S4(x - y). The spacelike projection operator can be removed if a term proportional to is in-troduced. However, the definition of S in equation (l) allows us to absorb these extra terms in S. We therefore, find -—T(x,y;n) = Su{x;n)64{x-y). (2) This can be integrated if S is curlless, that is, if 8 S Gross and Jackiw 2 have shown that equation (3) is always satisfied if the equal time commutator of A(x) and B(y) is considered to be the limit as x 0—>yo of the unequal time commutator of A(x) and B{y). We will see in the next section that the B J L limit allows us to calculate equal time commutators this way. After integrating equation (2) we finally obtain J n where r 0(x,y) is an arbitrary Lorentz covariant term. This equation shows that the T product is covariant if there are no Schwinger terms in the equal time commutator of A and B. It is easy to extend our analysis to the case of three operators. We define the covariant T* product and the seagull r by T*(x, y, z) = TA(x)B{y)C(z) + r (x, y, z). Following a procedure similiar to the two operator analysis we obtain 6 -—r(x,y,z;n) = 64{x - y)TS^B(x;n)C(z) onv + 64(x-z)TS»c(x;n)B(y) + 64(y-z)TS»BC(y;n)A(x) where S^B is the Schwinger term in the commutator of A and B. This equation can be integrated if the right hand side is curlless. It has been shown 2 that the curlless condition is satisfied if A, B, and C satisfy the Jacobi identity. But, as we will see later, the Jacobi identity sometimes fails. Before we look at these failures we must discuss the B J L limit. 3. The Bjorken-Johnson-Low Limit The BJL limit is a relation between equal time commutators and time ordered products and allows us to calculate the commutator from the Feynman diagrams of perturbation theory. Consider the matrix element of the T product of operators A and B between arbitrary states, T{q) = j d4xeiqx(a\TA(x)B{0)\P). To derive the BJL limit we use the integral representation of the step function du e~ixoU 8(x0) = j 27T U + It and write T(q) in terms of the spectral functions and This results in Now let qo —*• oo for fixed q to obtain ,{q) = J d4xeiqx{a\A{x)B{0)\(3) i{q) = j d4xeiqx{a\B{0)A{x)\f3). dq'o \ p(q'0,q) p{g'o,Q) Qo - q'o + *c qo - Q'O - I E . lim T[q) = — [ ^[p{q'0,q) - p{q'0,q)] oo q0J 27T 3 / TZV'O[p{q'o,q) - P{%,q)] q&J 27r 9o + qo. + = — I dzx€-i?£(a\[A{0,x),B(0)]\p) QoJ - \ ! d3xe-iq-s(a\[A{O,x),B{O)}\0) Qo J + ••• . Johnson and Low3 have shown that the commutator of A and B is logarithmically divergent if the expansion of T(q) at large qo contains terms of the form ^ log go- Sim-ilarly, they have shown that the commutator is quadratically divergent if the expansion contains terms of the form qo log qo = -~qo log qo-5 In perturbation theory we calculate the covariant T* product and not the T prod-uct. The difference between T and T* is the seagull and in position space it depends on a delta function and possibly derivatives of delta functions. In momentum space the difference is a polynomial in <7o- Thus, to calculate T from T* we let qo —> oo at fixed q and drop all polynomials in qo- This technique is illustrated in the next section where we look at a commutator anomaly in QED. 4. The Vector Current Commutator in Quantum Electrodynamics The time and space components of the vector current j M = t/ry^t/i in QED exhibit some interesting commutator properties. If we calculate the commutator by simply using the canonical commutation relations we get the result [j°(t,x),f(t,y)} =0. (4) It is easily seen that this result cannot be correct. First, take the vacuum expectation value of equation (4) and differentiate with respect to yl. Then use current conservation to obtain (o\[j0(t,x),d0j0(t,y)]\o) = 0. Next, write doj° as i [ /T, /°] and insert a complete set of eigenstates of the energy. Taking the limit y —> x, we finally obtain £ ( £ n - £ o ) | < 0 | / ° ( x ) | n > | 2 = 0. (5) n Since (o|/°(x)|n) cannot be zero for all excited states, the left hand side of equation (5) must be greater than zero. Canonical reasoning therefore fails in this example. But the BJL limit allows us to find a different value for the commutator. The T* product of and /" , ^v{q) = j d4xeiqx(0\T*j'i{x)jl/{0)\0 6 is given to one loop order by Fig. 1, f d4p J (2TT)4 tr 1 "7 m + ie — — m + ie This integral is solved using the Pauli-Villars regularization4. The result is where f(r2) te STY In _ i f ! 2 f m2 3nq /4 dr f{r2) 4m= r2(r2-q2) 1 + 2m2 1 - 4m2 (6) r" I v and A —» oo. The terms containing In ^ are seagulls and can be ignored in our calculation. We handle the terms containing the integral by noting that and defining so that lim f(r2) = l + 0(r~4) g(r2) = f(r2)-l lim g{r2) = 0{r-4). We can now write ' O O Um* r2(r2-q2) J4rn2 r •oo ,2 / J .2 m oo J Am- r JA ' 4 m - ' ' 4 m 2 r2 — <72 4m2 and take the limit go —• oo, lim 9' • M r . / 4 m 2 r 9 0 Umi q o — o o y 4 m 2 r 2 (r 2 - g2) _ l n _ ? L + i ^ + ? ; + 0 ( , - ) . 4m2 qi qi Inserting this into equation (6) and dropping all seagull terms results in „-„2 lim q0T°*(q) = ~ go —>oo Ait /•oo n2 - / dr 2 f f(r 2) J Am-37T go—•oo 4m^ i^2 Fig. 1 One loop diagram for T' From this we finally obtain <0|[j°(0,f),iI(0)]|0) = - ^ - 4 m 2 - / <fr2<,(r2) c9t<53(f) 37T i f ! 37T (Jo —*oo + ^ lim c 7 2 l n ^ ^ 3 ( £ ) °~ ~ — Am1 it + —dlV'66(x). The commutator calculated with the B J L limit contains a single derivative of a delta function whose coefficients are a quadratic divergence and finite terms. There also is a triple derivative of a delta function with a finite coefficient. The difference between the B J L limit value and the canonical value is one kind of commutator anomaly. The discussion of our other kind of commutator anomaly, the Jacobi identity failure, will have to wait while we look at the BJL limit for double commutators. 5. The Bjorken-Johnson-Low Limit for Double Commutators The B J L limit for double commutators is derived by an extension of the method for the single commutator BJL limit. The result is lim lim q0PoT(q,p) = - f d3xd3yeiqseip~»(a \B{0,y), [A(0 , z ) ,C(0 ) ] l /? ) o—•ooc/o—*oo J \ L J / Po where T(q,p) = j d4x d4y e i q x e i p y {a\TA{x)B{y)C{0)\P). The order of the limits is important. If the order is reversed the B J L limit becomes lim lim qop0T{q,p) = - f d 3 x d 3 y e - i q x e - i M ( a \A{0,X), [B(0 ,y ) ,C(0 ) ] l fi). (jo—*oo Po—»oo J \ L J / As in the single commutator case the T product is obtained from the T* product cal-culated in perturbation theory by dropping all polynomials in po and qo. With this for-mula in hand, we can now look at the Jacobi identity failure. 9 6. The Jacobi Identity Failure To test the validity of the Jacobi identity for two vector currents j M = ipi^ijj and one axial vector current j£ = Vn^lsi/J in QED, we must calculate J^a(Q,p) = J d3xd3y ^(0,x),[r(0,y),j5a(0)] >(0 ,y),[i B a(0),y*(0,x)] i 6 t t(o),[y*(o >x),y(o,y)] and see if it is zero or some other value. Each of the terms of J^wa is obtained from the double BJL limit; / d3xd3ye-^se-iPy(0 '^(0,x),[r(0,y),i5Q(0)]]|o) - lim lim q0p0Ttlva{q,p), (7) g0—»oo po —»oo j d3xd3ye-lf*e-*f(o\ [j"(0,y), [i 5 a(0),^(0,x)]] |o) - lim lim q0PoT^a{q,p), (8) po—>oo g0—*oo and j d3xd3ye-i^e-^y{o\[j^(0), [j»(0,x),r(0,y )]] |o) = - lim lim q0k0T^a(q,-q - fc) (9) fc0—»oo go—'oo where T^a{q,p) = J d*xd4ye*-xei'-v(0\Tj'l(z)j''(y)j?(0)\0) and fc = —(q + p). The diagrams in Fig. 2 are the lowest order contributions to the covariant time ordered product. The sum of the two contributions is — 7 ~ 7 f — — m-]- it i — m + it /+ p1 — m + it " 7 7 5 10 Fig. 2 One loop diagrams for T' 11 Rosenberg 5 has solved this integral. The result is ~ T ^ ( q , p ) = q ^ a [q • phx{q,p) ~ p 2 [/2 0(?,p) - ho(q,P)} - Pj3EP>xua q-plu(p, q) - q2 [ho(p, q) ~ ho{p, q)] - p 1 / g p P ^ e ^ a [ j 2 o ( 9 , p ) - / i o ( g , p ) ] + q^qpp^a[l20{p,q) - I10(p,q)] + Ql/qPPf3ep^aIn(q,p) -T^qpPpe^hxM (10) where Ist{q,p) = dx dy—— Jo Jo y l 1 y)q2 + x(l — x)p2 + 2xyq • p — m2 To calculate the right hand side of equation (8), we first do the y integration in Ist and then expand the remaining integrand in powers of qo, dropping any seagull terms as we proceed. For Iso{q,p) this results in so{q,p) = Jo dxxs - ~ + 2xPf3+0(q^) ln x(l — x)p2 — m1 ql ( i i ) The logarithm in the integrand can be written as I n 4 + l n 4 + ln xn2 p2 x(l — x) 7.— x(l — x)—^ Po Po so(g,p) = / JO We can now expand the third logarithm in the above expression in powers of po and after dropping a few more seagull terms we obtain dxx* [ - 1 + 2x% + O(qo-4)} [in 4 - ^ " T T - l ~K + °(Po4) • . 0 0 9o J L m Po x ( l -x) Po Upon examining equation (10) and our expansion of Iso(q,p) we see that those terms in equation (10) proportional to qpEp^p2 are either seagull terms and do not contribute to T^VOc or are zero when the limits in equation (8) are taken. There is, however, a non-zero result for some of the terms proportional to puqpppEp®iX°c. When 12 the other Ist integrals are expanded in a similiar manner we find that none of them give a non-zero value for the right hand side of equation (8). The result we find for the right hand side of equation (8) is —9 £ * Pi IT* lim p2 In 6 Po—»oo m2 — m ^ 2 ~P Equations (7) and (9) are calculated in a similiar manner and we finally obtain it J^a(q,p) = ^g»0el0™ql 7T 7T' 1 i - 2 i ?0 2 1 - 2 - hm q0\n—-m - -q 0 qo-»oo mz 6 1 r 2 i Po 2 1 - 2 - hm p 0 In — - m - - p 7T £ lim fc02ln^ o k„—>oo in1 6 m k The Jacobi identity failure for the massless theory has been analysed by Levy 6 . In his analysis he encounters some ambiguous terms. To see how these ambiguities arise we expand the logarithm in equation (11) for m = 0, In x(l — x)~ P2 In x(l — x) + In — In <7o P*_ m2 The In 4 term can be interpreted in several different ways depending on how we choose to define the limits. For the appropriate definition of the limits it can even be made to disappear. This ambiguous term becomes in our theory a quadratic divergence. The Jacobi identity fails if one of p, v and a is zero and the other two components are spatial and unequal. When this condition is satisfied, J/^** j n position space con-tains a single derivative of a delta-function whose coefficients are a quadratic divergence a and a term proportional to the square of the mass. It also contains a triple derivative of a delta function with a finite coefficient. We have seen that the Jacobi identity does fail. In the conclusion we will attempt to answer the question—why? 13 7. Conclusion Are the anomalies we have discussed a part of the theory itself or are they due solely to our method of calculating the commutators? It is possible that the anomalies occur because we worked to lowest order in perturbation theory; if the entire pertur-bation expansion were summed then perhaps the anomalies would disappear. Perhaps the failure lies with the BJL limit itself. But we showed without the BJL limit, from elementary considerations, that the vector current commutator in QED does not main-tain its canonical value; it cannot be zero. Maybe the answer is that the BJL limit value and the canonical value are completely unrelated, that they are entirely different objects. If this were the case the BJL limit would still be useful since it provides, through the sum rules, an experimental means of measuring commutators. A connec-tion between the anomaly in the axial vector Ward identity and the non-canonical value of the vector-axial vector commutator calculated with the BJL limit has been found7. It is the Schwinger term in the commutator which causes the anomaly in the Ward identity. No connection has been found for the vector-vector commutator nor for our Jacobi identity failure, but future work may help us discover a connection and then the theory and the BJL limit might someday be consistent. R e f e r e n c e s 14 1 J. Schwinger, Phys. Rev. Letters 3, 296 (1959). 2 D. J. Gross and R. Jackiw, Nucl. Phys. B14, 269 (1969). 3 K. Johnson and F. E. Low, Prog. Theoret. Phys. (Kyoto), Suppl. 37-38, 74 (1966). 4 C. Itzykson and J. Zuber, Quantum Field Theory, (McGraw-Hill, New York, 1980). 5 L. Rosenberg, Phys. Rev. 129, 2786 (1963). 6 D. Levy, Imperial College preprint, (Feb. 1986). 7 S. L. Adler, in Lectures on Elementary Particles and Quantum Field Theory, ed. S. Deser, M. Grisaru, and H. Pendleton, (MIT Press, Cambridge, Mass., 1970);R. Jackiw, in Lectures on Current Algebra and Its Applications,ed. S. Treiman, R. Jackiw, and D. Gross, (Princeton University Press, Princeton, NJ, 1972). 

Cite

Citation Scheme:

        

Citations by CSL (citeproc-js)

Usage Statistics

Share

Embed

Customize your widget with the following options, then copy and paste the code below into the HTML of your page to embed this item in your website.
                        
                            <div id="ubcOpenCollectionsWidgetDisplay">
                            <script id="ubcOpenCollectionsWidget"
                            src="{[{embed.src}]}"
                            data-item="{[{embed.item}]}"
                            data-collection="{[{embed.collection}]}"
                            data-metadata="{[{embed.showMetadata}]}"
                            data-width="{[{embed.width}]}"
                            async >
                            </script>
                            </div>
                        
                    
IIIF logo Our image viewer uses the IIIF 2.0 standard. To load this item in other compatible viewers, use this url:
http://iiif.library.ubc.ca/presentation/dsp.831.1-0085250/manifest

Comment

Related Items