on the transition matrix and the green function in the quantum
TRANSCRIPT
Progress of Theoretical Physics, Vol. 10, No.6, December 1953
On the Transition Matrix and the Green Function in the Quantum Field Theory
Sho TANAKA and Hiroomi UMEZA W A
Institute 0/ Theoretical Physics, Nagoya University
(Received July 26, 1953)
617
The J. Schwinger's formalism of the Green function in the quantum electrodynamics is applied to the transition problem of the state. It is shown that the many body kernel in the Heisenberg representation involves the information about the transition of the state and this is dh'ectly represented by the repeated use of the one body kel'Oel G,@ and the vertex opel'ator rlL defined by J. Schwinger. Further, the renormalization is discussed without use of the usual perturbation theory, although then: remains the difficulty associated with the b-divergence.
§ 1. Introduction
The propagation of the interaction effects between the fields is usually represented by
the Green functions in the present quantum field theory. In the interaction representatioq
these Green functions are the well-known dB, SF. etc. The matrix describing the transi
tion of the state is constructed by the repeated use of these Feynman's functions. As
was shown by Stiickelbergl), introducing the Feynman's functions and the usual Dyson's
S-matrix follows as a logical consequence of the requirements of the c:ausality for the
propagation of the interaction effects. This fact suggests that the Green .function is one
of the fundamental basis of the current quantum field theory.
The importance of these Green function becomes dearer in the Heisenberg representa
tion, because there the state vector is time-independent and the temporal development of
the system is described by the field operators and $0 it can be expected that the Green
function involves the information about the transition of the state. On the other hand,
many authors2) ,3) have expected that the Green function of the 1z-body problem involves
also the information about the stationary state of the nobody problem.
It is the aim of this paper to investigate the detailed property of the Green function
in the Heisenbeg representation. A crucial method to treat the Green function in the
Heisenberg representation ,has been proposed by J. Schwinger.2) In this paper we shall
treat our problem along the same line as he has done and restrict ourselves' only to the
quantum electrodynamics.
In the usual perturbation theory, the Green function of the one body problem has
a special importance. As Dyson4l has shown in the quantum electrodynamics, the S-matrix
element is obtained through the substitution of S;., D;', and r for the electron line, photon
line, and the vertex part in any possible irreducible graphs corresponding to the given
transition process.
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618 s. Tanaka and H. Umezawa
These S~, D~ correspond to the Green functions of the one body problem. In § 4,
we show, without use of the usual perturbation theory, that the mattix element of any
transition is written by an adequate graph which contains the Green function of the one
body problem and J'~ as for the internal line and vertex part, respectively. Further, we
will treat the renormalization problem in our method without use of the perturbation theory.
However, on account of the difficulty associated with the b-divergence, the completion of
the discussion is confined to be left in future.
§ 2. On the transition matrix and the Green function
of the many body problem
We treat the problem in the quantum electrodynamics, whose Lagrange density IS of
the form
L= -1/2 ·Sb{r~(i1~-ieA~) +x} if'+ 1/2· {Sb~+~if') +h.c.
-1/4.F~~.1/2· (a~A~)2 -J~A~, (2·1)
where '1) is a spinor source which anticommutes with if' and Sb, ~ IS given by '1)*r4 and
J~ is a c-number source current and further F~"=a:LA"-a"AiJ..*
From (2.1), the well-known equations of motion in the Heisenberg representation are obtained:
{r~(aiJ.-ieA~) +x}if'='1),
o A~=-J~-j"", j',l- = -ie/2 h~if'+h.c.
(2.2)
(2.3)
(2.4)
Now let us introduce the following notation -for the operators in the Heisenberg representation, A(xJ), B(x2), ••• ,
(2.5)
where 1JY0 is a vacuum state vector defined as the minimum energy state in this representa
tion. Further, we use the interaction representation which coincides with the Heisenberg
representation at a (x) = 0 and denote the minimum energy ,state in this repre.sentation
as (/)0. If the quantities in the Heisenbergrepresentation, are denoted by ...4 (XI) , B(x2) , ... , corresponding to A (XJ ) , B(X2) , ... , respectively, then there are following relations between both quantities:
...4(XJ) =U(a(x1), 0)A(X1) U-\a(x1) , 0), etc. (2.6)
As Gell-Mann and LowE) has shown, 'Fa may be written as
1JY0=.!.U-\±CXl, 0)(/)0/((/)0' U-1(±CXl, 0)(/)0), (2· 7) c
where c is a normalization constant.
* The stat expresses the hermitian conju&ate.
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Oil the Transition Matrix and the Green Function in the Quantum Field Theory 619
Using (2.7), (2.5) is rewritten as
(A(x1), B(X2) , ... ) + = ($0' U( 00, O)P(A (%1)' B(x2) , ... )
xU-I(-ex:., 0)$0)/($0, U(OO. -00)$0)' (2·8)*
where we used the following relation;
U(a, 0)U- 1 (a','0) =U(a, a'). (2.9)
Since the annihilation and creation of a-patticle are described by the positive and
negative frequency parts Q!(x) of a-field operator Q~(x), respectively, we have from
(2.8) the next theorem. Namely, the transition matrix .s~ between the initial state,
where a-particle with the energy-momentum klL and spin state r etc. exists, and the final
state, where a-particle with the energy-momentum k: and spin state r' etc. exists, is
5 r..t(k/, r; ... )(Q (-). a () ) fi=aL< i(k , ..... ) a. Xl , ... , ~" ;rl , ... +,
J.I.' , (2.10)**
where F1~:::5 is the operator which takes out the Fourier's amplitudes refering to "k lL ,
r and the negative frequency part at the world point -Y1 " and "k:, r' and the
posi~ive frequency part at the world point Xl'" a is a normalization constant and ;r1 and
Xl are the coordinates of the particles in the initial and final state, respectively, and so
their time components are -;;- 00 and + 00, respectively. If we bring out the quantities
of Xl in front of tpe one of .:!'·l' we have the following relation:
(Qa.(;rj),"" Qa.(.i)···)+=($o' Q,,(,1;·l)'···' U(oo, -OO)Qa.CX1)···$0)
x 1/($0' U(oo, -00)$0)'
which gives the proof of (2. 10) . Using the the creation and annihilation operators q;, the Fourier transform of Qa. is
expressed in the form
Q,,(x) = lim ~ V-l/~[d"r(k)q: (k)exp i(kr-kot) p-)om k
+ d,.*,.(k) q;: (k) exp -i (kr- kot) ]. (2.11 )
The normalization constant in (2· 10) is expressed by the reciprocal of the product of
* If we denote the interaction Hamiltonian density as H(x) and apply the usual perturbation theory, we have
(2·8)'
The appearance of the denominator in (2·8)' corresponds to the procedure in the usual perturbation which leaves out of consideration the isolated diagram, whose init'al and final states are the vacuum states.
** (2·10) has been applied to the problem of the multiple production of meson; H. Umezawa et aI., Phys. Rev. 85 (1952), 505.
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620 S. Tanaka and H. Umezawa
(d .. t;(k') ...• d .. r(k) ... ).*
Now we define the Green functions for many body problems as follows: electron Green functions
GYj(Zlt zD = al(7)(zD(cfJ(Zl»'
G~(Zl' Z2' z1) = ala~(Z2)(cfJ(Zl)' ¢(zD )+E,
GYj(Zl'X~, z~) = alar;(X~)(cfJ(Xl)' ¢(zD )+E,
GYj(Zl' X2• z~,z~) = al(7)(xD (cfJ(zl),¢(zDcfJ(Z2»+€ etc.
photon Green functions
<MJ.~(~l' ~2) = alij~(~2)(A(J.(~1»' <MJ,~,G(~l' ~2'~3) =a/ij~(~3)(A(J.(~1)' AG(~2»+'
mixed Green functions
K~T,~(Zl' z~, ~1) = a/aJi~l)(cfJ(Zl)' ¢(ZD)H
KYjJ.~(Xl' x~, ~1' ~D = a/aJ~(~D (cfJ(Zl)' ¢(z~), A(J.(~l) )+.
According to the calculation rule given by J. Schwinger, we have
GYj(Zl' zf} =i(cfJ(Zl)' ¢(x~) )+E-t'(cfJ(Zl» (¢(x;),
G~(Zl' X2' z~)=i(cfJ(z]), ¢(X;) , 1'(Z2»+E
-i( cfJ(xt ), ¢(xD) + (1' (Z2) ) E,
KtjJ(Zl' x;, ~])=i(cfJ(ZI)' ¢(.xD, A(~l»+E
-i(A(~]»(1'(Zl) ¢(xD )+E,
(2.12)**
(2.13)
(2 ,14)
(2 ·15)
* (2 ·11) for the case of the field with the arbitrary SpIn has been discussed by Y. Takahashi and H. Umezawa; Prog. Theor. Phys. 9(1953), 14.
** E in the expression ( >+ E means the sign function as to the coordinates appearing in ( >+. For
instance, for the case of (I/>(x), I/>(X2)' if(x/), ¢(xl)+>E, E is given by
E = E (xli x2) E (x/, ;)(1l) E (X1o xl) E (x2, x/) E (x9' xl) E (X1o x'),
where E (x,y) = 1 for Xo >yo,
= -1 for xo<Yo.
In th~ fo110',,:n6 discu~sion W~ shall eliminlte this symbol as far as it does not give rise to mistake.
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On the Transition Matrix and the Green" Function in the Quantum /i"ield Theory 621
Since U(a, a') has non vanishing matrix element only for the transition satisfying
the charge conservation law, we have the following relation for F, in which the numbers
of the¢ and (jj are different each. other ;
(2-·16)
For example, we have
(2.17)
From the invariance of the theory under the charge conjugation, we have the Furry's
theorem, (AfL)J-+o=O. From these relation and (2. 10), (2· 15), we find that the many body Green function
at the limit <'1--,>0, ~--,>O} corresponds to the transition matrix element. Hereafter,we
denote these quantities with (J--'>O, ~--,>O) by those with the super-suffix 0.* For example,
G~(:.rr:r2'i'tx2)' @Ailill2),andKTjo,(x1xtl2} correspond to the Moller scattering of the
two electrons, photon-photon scattering, and Compton-scattering, respectively.
On:e body Green functi()n is connected with the current J;, (x) as follows:
(2.18)
where
GTj(x; x) == lim [GTj(x, x') +GTj(x', x)J/2. X'-»Z
(2·19)
Hereafter, the matrix representation for the coordinates of electron and photon is used and
so the matrices 1, a", ¢, (jj, A",. GTj and @J.~ are 8(x-x'), 8(x-x') a". ¢(x)8(x-x'), (jj(x)8(x.-x'), A,,(x)Q(.i'-X'), GTj(x, x') and @J.~(x, x'), respectively.
From the equations of motion (2·2), (2·3), we have for GTj' @J.~ the equations,
{r fL (a fL -ie(A,,») + M} G~='1 +ier~ (¢·)8 / ij~ «(jj),
{o- P} @J.~=·8,,~ 1.
(2.20)**
(2.21)
In the above expression the mass operator M and polarization operator P are the matrices
whose elements are given by M(r, x'), P (f, f') defined as follows:
J dx"M(x, x")GTj(x", x() = (x-er,,8/ijfL(X»GTJ(x, x'),
J d~IlP (f, f")@J.~(f", fl) = eTr{r,,8/ijv(~I) G.~(f, f)}.
(2·22)
(2.23)
* The limiting process (J ---+0, 1)---+0) should be taken after the variational operation of (2 ·12), (2 ·13) and (2·14).
** The product of the two matrices A and B is defined by'
(X\AB\x')=~ dy(.riA\y)(y\B\x').
FUtther the symbol . in the expression A· or ·A denotes the right or left cooroinateof the matrix A.
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622 S. Tanaka and H. Umezawa
As was shown by J. Schwmger, we have
aiaJ"(~) GY)IJ,Y)+o=eG~I de r~(e) G~@~.~(e ~),
where the vertex operator r~ (~) is. defined as foIlows2) :
From (2.22) and (2.24), we have
and so
M:-x1 +ier",(A",)- e2r", J de·G'ljr~(~')@J,~(~',.) -er[1-'G'Ij a/a}[1-' {ie r~(¢:)aia./';,(¢)G~l} G'Ij'
§ 3. Note On the renormalization theory
(2 ·24)
(2.26)
(2·27)
In this section a short note on the relation of the above theory with Dyson's one
is given. The differential equation (2.21) can be transformed into the integral form;
where
G~(x, x') =5.1'(x-x') -axJ dy 5.1'(x-y) G~(J', x')
-J dydy' 5.1'(x-y) L]°(Y,Y') G~CY', .x'),
~O=MO-x'l, x'=x+ax.
Using (2·27) we have
G~(x, x') =SIl'(x-x') -ax J dy SF(X-y)G~(y, .x')
_e2 J dydy'dy"deSIl'(x-y)G~(J"Y') x r~(e ;y',y")G~(J'''' .x')@J,~(e=',y). (3·2)
If we replace G ~ by S; in (3. 1), this equation cor
responds to the integral equation given by Dyson and
(3.1)
Fig. 1
Fig. 2 (i)
Fig. 2 (ii)
L]0 amounts to the total contribution from the self-energy graph. (3 ·2) agrees with the
final integration of the self-energy graph given by Dyson and corresponds to Fig. 1, in which the electron line, photon line and vertex b correspond to G~, @J. and 1':, respectively.
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On the Transition Matrix and the Green Functio1z in the Quantum Field Theory 623
The fact that r of the point a is not replaced by r~ coorresponds to the Dyson's argu
ment on the b-divergence, because we must take into account only one of the equivalent
graphs (i), (ii) in Fig. 2.
In the quantum electrodynamics we can normalize cp and All- so that in the high energy ·region all possible quantities with dimension of the length are the momenta PII- of particies6)*. In this case the dimensions of G~ and @~ agree with those of SF and DF, respectively, and r~ and r II- are the dimensionless quantities.
Let us separate the infinite constants from G~, @~ and r~ as follows:
G~=Z2G~1'
@~=Zg@~,
(3.3)
where G~l> @~1 and r~l are free from infinity. Substituting (3.3) into (3.2), we have
G~(x, x') =~SF(X-X') -axJ dy SF (x-y)G~l(Y' x') Z2
-e~Z22Z1-1z:~J dydy'dy" derll-SF(X-Y) G~l(J', y') (3.4)
X !'HO(~' ;y', y") G~l(Y'" x')@~,~(~', x).
In the above equation, while the integrand of the third term is finite, its integration may
be divergent. Since this divergence comes from the contribution of the high energy region, the following discussion shows that this integral is at most linearly or logarithmically
divergent. Z1' Z2' and Zg are the function of the upper limit .p ~ co of the integration
concerning the internal momentum and so the dimension of the divergent Z1' Z2' andZg should be zero or negative power of the length. Therefore, the dimension of G~I' @~1
and r~l are [L-n] (n<.3, 1z<2, 11<0), respectively. Since the integral (3.4) is
most strongly divergent in the case of n=3, 2, 0, it is sufficient to treat this case for
the consideration of the highest degree of divergence. Then the integral has a dimension [D2-a-a-a-2J = [L], and can be written as follows:
f dydy'dy"derll-SF(X-Y) G~l(y,y')rs(e ;y',y")G~l(Y'" x')@J,.tce, x)
=Zll[A+B(rll-all-+ x) +C(rll-all-+ x)2+ ... ]
x J dySF(X-y)G~l(Y' x'), (3.5)
where A and B are linearly and logarithmically divergent and C is a finite quantity.
As Fig. 1 is symmetric in association with the two vertices a and b, it is expected that a infinite constant factor ~-1 appears from the vertex a as well as the vertex b after
* In the interaction. of the second kind, the situation is not so simple as in this case, because the coupling constant has the dimension of the length.
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624 S. Tanaka and H. Umezawa
the integration is analogous to Dyson's argument. However, the consistent proof of this
situation is not yet verified in our method. This defect which is due to the, asymmetrical
treatment of the two vertices makes it difficult to compare our method with Dyson's one also in the discussion of the skelton approximation in' the next section. *
Substituting (3· 5) into (3·4), we obtain the following relations asa necessary con
dition for the convergence of the right side of (3.4) :
Z2=1-ie12B,
e1=Zl-lZ2Z 31/2e .
(3.6)
Here eI and x' should be considred as a finite and observable electric charge and mass,'
respectively. Then (3.4) becomes as £ottows:
(3.7)
(3 .6) is in agreement with the condition as to the renormalization constant given by Dyson. Further it is easily found by the same dimensional argument as in the above
(3.5) that the divergent quantities are restricted only to self-energy parts G~. @~ and
vertex part r~. Therefore, the theory is entirely free from divergence, provided that it is shown that
any Feynman diagram of Smatrix is expressed by the irreducible skelton in which internal
lines, vertex, and charge correspond to G~1> @~J' r~l> and t'l' respectively. In this paper the method in which any transition matrix is represented entirely by the G~, @J. and [~ is called the skelton approximation. If we have the formulation of the skelton approximation, any vertex in Fig. 3 is of the form e( G~ @~G~)1/2r~ which can' be reo,
written as follows;
?-lZZl/2(G O ft1 0GO)1/2TlO _ . (Go ft1 0G O)r. ° e.61 2 3 "l)l \:!JJl"l)l 1 (L1- e 1 1}l\:!JJl"1)l ,.1, (3.8)
so that it turns out that there exists no more any infinite quantity in the theory.
Thus it is necessary for completion of our procedure only to investigate the possibility of the above skelton approximation and this is the aim of the next section. As will be shown there, unfortunately, we can not yet find the complete formulation of the skelton approximation and this problem is left to be investigated in future.
§ 4. The skelton approximation
In this section we shall prov.e that the transition matrix element is obtained through
substituting the Green function of the one body problem and r,. into any internal lines and the vertex part of the adequate graph corresponding to its process. However this
graph is not completely equivalent to the skelton and we must often use the uncorrected
* If this deffects are get rid of, one could set up a non-singular theory by using the lagl'angi~n gh'en by G, Takeda7) and applying the variational method in §2;
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On tlte Transition Matri% and the Green Function in tlte Quantum Field Theor), 625
vertexrll-' although it is needless to use SF and DE' According to (2. 10), it turns out that the problem is how to express all the many
body Green function by the one body Green function and the vertex function rll-; i.e.,
the corrected function approximation. In the following we discuss on this problem in some
examples, i.e., the Moller scattering of two electrons and the photon-photon scattermg. (i) Moflir scattering
According to (2. 10), the transition matrix element for the Moller scattering corres
ponds to G~(,:t:"l' <r2, z:, z;). Using (2·12), we have
G~(%l> %2' %{, %D=-J2la~(%~)a~{X2)G'I(XH %D1J'I"O (0)
+ G~(~l X 2 %~ %~),
where
-iG~(xl' %DG~(X2' xD·
This· is represented by the diagrams denoted in Fig. 3.
In this diagram and hereafter it should be noted that
the straight and waved line, the vertex and vertex with
circle correspond to G~, &1J, r 11-' and r~, respectively.
The second term of (4· 1) expresses two independent
electrons scattering without the real interaction. The
effect of the true Moller scattering due to the real
interaction of two .electrons is involved in the first terms
of (4·1). From (2.21), we have
Further using (2.17) and the Furry's theorem, we obtain
Substituting the following. relation
;(.,
(4·1)
(4·2)
Fig. 3
(4·3)
(4.4)
(4.5)
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626 S. Tanaka and H; Umezawa
into (4. 4), we have
(4·6)
where
(2) J G ('%2' %~) =_e2 [G~r(J.G'Il(%2') r(J.(f/) G'IJ'X~)@J(e,.) G'I)
+ G'IlrG'IlC" %DG"l(%2') J r(e)@Jce, . )G'IllIJ,'Il+O' (4·7)
This is represented by the diagrams in Fig. 4,
It can be shown that the second term of
(4, 6) contributes to the skelton higher than
the fourth order. Using (2,22), we have
and this diagrams correspond to e2-skelton.
lJ2 M lJ2 (MG G-1) lJ7} (%~) lJ7} (x 2) lJ1) (X;) lJ~ (x 2) 'I) 'Il
lJ [( lJ G )G-1] x-q(J.-·"I) 'Il . /J1)(x~)/J~(.t'2) lJj~,_
(4.8) Fig, 4
After the tedious calculation, (4, 8) is rewritten in the form;
;Y MI =-e G ~[G-l /J2G'Il ] G-11 . /J1)(%~)a?(X2) J,''1+0 r 'Ilij' 'Il a7}(%~)/J1)(.t'2) 'Il J,"l+O
(4.9)
Therefore, from (4· 6) we have
From (4.3), (2.17), (4.5), we can obtain the relation
(2)
where G is defined by the left side of (4,7) without superscript O. The second term of
( 4 .4) gives to (4. 10) the skelton higher than the e6-approximation, and we write this part
as OCe6). Using (4·10), we can rewrite (4.10) as follows:
(4.12)
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On the Transition Matrix and the Green Function in the Quantum Field Theory 627
The second term of e 4 . 12) corresponds to e4-skelton, and is given by
(4)
G~e ;x2, ,x~)
=-ie4G~rG~ [rG~eX2') f re~")G.,,@JC~"'·) f rC~")GC ,x~)@Jee, :)G"lC:')
This
+rG1)eX2') J rCf") G"lJ rce)G"IJ(,x~)@Jce,. )@Ae',:)G1)(:')
+rG."eX2') J re~")G''le,x~)@./C~'', :)G."C:.) J rce)G",@J(;'" )lJ,.,,~o
-ie4G~rG~rrG.,..(:,) J rc~") G ... e,xD@Jee:",· )G."eX 2') J rce) G.,,@J(e,:)
+rG.,,(:,xD G.,,(x2.) J r(~") G ... (,x~)@Ae',.) J rce) Gy/M ce,:)
+rG.,,(:,x~) G."eX 2') J ree') G.,,@J(e':) J l'(e) G'Ij@JW,') ]IJ,~.o. IS represented by the diagrams in Fig. 5.
A X K X )::( X
Fig. 5
e 4 '13)
As stated in the preceding section, it should be noted here that only some part of all vertices are replaced by r",. For instaric~ in Fig. 4, only one vertex among two is replaced by r",. Thus the contribution which corresponds to Fig. 6 in the usual perturba
tion theory is. not involved in this &agta:m, but in Fig. 5 which belongs to e4-skelton. Of course, if we takemto account infinitely
higher order terms in the present approl{rmation, then the both
vertices will be completely corrected and so by r"" and then the skelton approximation May be obtained. However such a procedure is of a perturbation t:heor~ticif{ concept. This unfavourable situation
of our method is due to the fact that, in the course of obtaining
the higher orderskdton by applying (2.24) to one body Green Fig. 6
function, .only one vertex among two of the self-energy part is replaced by {''''. (ii) Photon-photon scattering
Now we discuss briefly on the photon-photon scattering. This· transition matrix ele-
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628 S. Tanaka and H. Umezawa
ment corresponds to
( 4.14)
where (0)
@J(~lI ~2' ~3' ~4)=-i[@J(~l>'~2)@J(~3' ~4)+@J(~1' ~3)@J(~2' ~4)
+@J(~l' ~4)@J(~2' ~3)J· (4.15)
This is represented by the diagrams in Fig. 7. After the analogous calculation as for a~ .
--. G~I' 'the first term IS trans-a'1)a~ ". formed into the following form:
a2@ I ij(~4) ij(fs) J->O
= -@~ ij(~;~J(~3) L~9@~' (4.16)
J" Fig. 7
(4.17)
Further, we have
a3 G.'1 ij·aJ( f 4) a I( ~3)
(4 ·18)
where the symbol (x---7:J!) means the term obtained by the exchange of X and :JI in
the preceding term. Thus the final result is given by
(4.19)
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On the Transition Matrix and the Green FUllction in the QuantuJn Field Theory 629
where (4)
@~(" '~3' ~4)
=-ie4@~T,.[rG"lS r(e)@J(~/, ~4)G'/jf r(~")@J(~",.)GYjf l'(~"')@J(~'''' ~3)GYj
+rGYjf r(~')@J(~" ~4)GYjf r(~") @J(~'" ~3)G'/jf {'(~"')@i~"',· )G'/j
+rGYjJ rW)@i~', ~3) G'/jJ r(~") @A~",·) GYjf r(~ ")@(~"', ~4) GYj'J.Yj"o
+ (e:4-~)' These correspond to e4-skelton approximation and are represented by diagrams in Fig. 8.
Fig. 8
All other processes be treated in the similar method as to the above two examples.
The authors express their appreciation to Professor S. Sakata for his kind and helpful
interest and his continual encouragement and also thank to Mr. R. Kawabe and Mr. S.
Kamefuchi for their valuable discussions. Their thanks are finally due to Professor M.
Kobayasi for the hospitality to one of them (S.T) at Yukawa Hall.
References
1) E. C. G. Stiickelberg and T. A. Green, Helv. Phys. Acta 24 (1951), 153. 2) J. Schwinger, Proc. Nat. Acad. 37 (1951), 452. 3) E. E. Salpeter and H. A. Bethe,Phys. Rev. 84 (1951), 1232. 4) F. J. Dyson,Ph},s. Rev. 75 (1949), 1736. 5). M. Gell~Mann and F. Low, Ph}, •. Rev. 84 (1951), 350. 6) S. Sakata,H. Umezawa and S. Kamefuchi, Prog. Theor. Ph},s. 7 (1952), 377. 7) G. Takeda, Prog. Theor. Ph},s. 7 (1952), 359.
Dow
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