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On How QCD Gauge Invariance Gets Realized in the Context of Effective Locality.

1. Introduction

In some recent articles [1-5], a property, which bears on the nonperturbative fermionic Green's functions of QCD, has been put forth under the name of effective locality (EL). This property can be summarized as follows.

For any fermionic 2n-point Green's functions and related amplitudes, the full gauge-fixed sum of cubic and quartic gluonic interactions, with fermionic loops included, results in a local contact-type interaction. This local interaction is mediated by a tensorialfield which is antisymmetric both in Lorentz and color indices. Moreover, the resulting sum appears to be fully gauge-fixing independent, that is, gauge-invariant.

This is an unexpected result because integrations of elementary degrees of freedom ordinarily result in highly nonlocal structures. The "effective locality" denomination, which sounds like an oxymoron, accounts for this unusual circumstance. It is worth pointing out that in the pure euclidean Yang Mills case and up to the first nontrivial orders of a semiclassical expansion, effective locality was observed as a welcome property in an attempt to construct a formulation dual to the original Yang Mills theory [6-8].

Now, apart from a supersymmetric extension, QCD is not known for possessing any dual formulation and the full EL functional expressions certainly attest to this difficulty. It remains that, like in the pure Yang Mills situation of [6, 7], the EL property may allow one to learn something about the nonperturbative regime of QCD and this from first principles.

In the next section a comparison of the QED and QCD Green's functions generating functional is given, while Section 3 displays the property of effective locality in the simpler situation of eikonal and quenching approximations where it was first noticed and then in full generality. Eventually, Section 4 presents some concluding remarks.

2. Contrasting Generating Functionals

In QED it has been known for quite a long time that manifest covariance and manifest gauge invariance are competing aspects of a generating functional construction. For short, starting from a photonic Lagrangian density of

[mathematical expression not reproducible] (1)

and corresponding action (at [lambda] = 1),

[integral] [d.sup.4] x [L.sub.0] = -1/2 [integral] [A.sup.[mu]](-[[partial derivative].sup.2]) [A.sub.[mu]] + [lambda]/2 [integral] [([[partial derivative].sup.[mu]][A.sub.[mu]]).sup.2], (2)

one may use the "inconvenient" (in Fermi's words [1]) term of [([partial derivative] x A).sup.2] to generate any relativistic gauge (manifest covariance), treating, for example, ([lambda]/2) [integral] [([[partial derivative].sup.[mu]][A.sub.[mu]]).sup.2] as a kind of "interaction." Gauge invariance is then guaranteed by enforcing charge conservation: clearly not a manifest way.

The construction can be summarized through the following steps. Starting from the free-field case ([lambda] = e = 0), one has, with [D.sup.(0).sub.F[mu]v] = [g.sub.[mu]v][D.sub.F], (-[[partial derivative].sup.2])[D.sub.F] = 1, the free- field generating functional

[Z.sup.(0).sub.0]{j} = exp{i/2 [integral] j x [D.sup.(0).sub.F] x j}. (3)

Then one can proceed in Schwinger's way with the "gauge-interaction term":

[mathematical expression not reproducible], (4)

with

[D.sup.([zeta]).sub.F[mu]v] = [[g.sub.[mu]v] - [zeta][[partial derivative].sub.[mu]][[partial derivative].sub.v]/[[partial derivative].sup.2]] [D.sub.F], [zeta] = [lambda]/1 - [lambda]. (5)

The full Green's functions generating functional now reads as ([lamba] [not equal to] 0, e [not equal to] 0)

[mathematical expression not reproducible] (6)

with (the phase factor appearing in the second line of (4) is absorbed into the normalization constant N)

[G.sub.F][A] = [[[gamma] x ([partial derivative] - ieA) - m].sup.-1], L[A] = Tr ln [1 - ie[gamma] x [A.sub.SF]], [S.sub.F] = [G.sub.F][0]. (7)

This is the standard Schwinger solution for the QED generating functional. For any polynomial and/or exponential functional F[A], the following differential functional identity holds:

[mathematical expression not reproducible] (8)

with the so-called linkage operator

[D.sup.([zeta]).sub.A] = -i/2 [integral] [d.sup.4] x [integral] [d.sup.4] y [de;ta]/[delta]A(x) x [D.sup.([zeta]).sub.F](x - y) x [delta]/[delta]A(y). (9)

This identity can be used to write eventually

[mathematical expression not reproducible]. (10)

Of course, this is the QED generating functional that would result from linear and covariant gauge fixing of (-1/2(1 - [lambda]))[([partial derivative] x A).sup.2]. However, [lambda] = 1 cannot be chosen as [D.sup.([zeta]).sub.F.[mu]v] would not be defined. It is at [lambda] = 1 though that manifest gauge invariance is maintained. As a result, Green's functions cannot display gauge invariance. As shown in (10), the bare photon propagator remains explicitly gauge-dependent, and through Ward-Takahashi identities, its radiative corrections are checked to be gauge-invariant. For the whole set of physical processes described by QED, the LSZ reduction formula and equivalence theorem [9] allow one to pass from nongauge-invariant Green's functions to gauge-invariant S-matrix elements. Recovering gauge invariance is therefore a circuitous procedure and it seems that the nonabelian structure of QCD offers a different possibility.

In the case of QCD, the same canonical steps canbe taken. To sum up and within concise notations (color degrees being understood)

[mathematical expression not reproducible], (11)

where the following propagator, of course, does not exist:

[mathematical expression not reproducible]. (12)

However, in QCD, unlike QED, one has

[mathematical expression not reproducible], (13)

that is, omitting fermionic variables momentarily,

[mathematical expression not reproducible]. (14)

Now, simply adding and subtracting a linear covariant gauge-fixing term of (1/2[zeta])[([partial derivative] x A).sup.2], it is elementary to proceed and pass from an undefined [D.sup.(?).sub.F] to the well-defined and covariant propagator [D.sup.([zeta]).sub.F]:

[mathematical expression not reproducible] (15)

and to a Green's function QCD generating functional of

[mathematical expression not reproducible], (16)

where fermionic dependence has been restored and the differential functional identity (8) used again.

However, likewise, adding and subtracting a gauge fixing of (1/2[xi])[(n x A).sup.2], with n being a lightlike vector, [n.sup.2] = 0, one gets (in the limit [xi] [right arrow] 0, [9])

[([D.sup.(n).sub.F]).sup.ab.sub.[mu]v](K) = -i[[delta].sup.ab]([g.sub.[mu]v]/[K.sup.2] + i[epsilon] - [K.sub.[mu]][n.sub.v] + [K.sub.v][n.sub.[mu]]/([K.sup.2] + i[epsilon])(K x n)) (17)

and a Green's function QCD generating functional of

[mathematical expression not reproducible]. (18)

As many identical forms as desired can be obtained for [Z.sub.QCD][j, [bar.[eta]], [eta]], differing only in the intermediate gluonic field function, [D.sup.(n).sub.F], [D.sup.([zeta]).sub.F], and so forth.

In conclusion, the following points can be proposed.

(i) In QED (where [lambda] = 1 cannot be chosen), these standard functional operations amount to a quantization in a given covariant gauge. Manifest Lorentz covariance is maintained while manifest gauge invariance is not. Gauge invariance is the matter of indirect recovering.

(ii) In QCD, surprisingly and explicitly due to the nonabelian structure, manifest Lorentz covariance and manifest gauge invariance can be preserved at a time.

(iii) Since no gauge fixing is really achieved, none of the several forms of the QCD generating functional, with [D.sup.(n).sub.F], [D.sup.([zeta]).sub.F], or any other free-field function, do indeed correspond to the usual QCD generating functional in the associated gauge.

(iv) There is but one possibility. Gauge field functions (i.e., propagators) must show up as necessary intermediates and not affect the fermionic momenta of the QCD generating functionals (16) and (18).

(v) Now, this is guaranteed by the property of effective locality.

3. Effective Locality

The property of effective locality will be first displayed in a simplified situation corresponding to the use of eikonal and quenching approximations.

3.1. Effective Locality in a Small Example: Eikonal and Quenching Approximations. With the help of the representation [10],

[mathematical expression not reproducible] (19)

any [D.sub.F]-dependent form of [Z.sub.QCD][j, [bar.[eta]], [eta]] can be used; for example,

[mathematical expression not reproducible]. (20)

However, representation (19) breaks the manifest gauge invariance. This can be remedied either by gauging the [chi]-field [6,7] or by means of an exact integration of the [chi]-field dependence. In the latter instance, the powerful Random Matrix theory allows one to do it in the "small case" at least [4]. So long as gauge invariance is concerned, however, none of the above possibilities is necessary as effective locality brings about a remarkable simplification.

Let there be a Fradkin's representation of the functional [G.sub.F][A] [11]:

[mathematical expression not reproducible], (21)

where u(s) is the 4-vector Fradkin's field variable, the subscript + stands for s-Schwinger proper-time ordering, and h([s.sub.1], [s.sub.2]) = [[integral].sup.s.sub.0] ds' [THETA]([s.sub.1] - s')[THETA]([s.sub.2] - s'). This representation is exact but fairly involved. In eikonal approximation (u(s) = sp) the ordered exponential reduces to

[mathematical expression not reproducible]. (22)

In (22), the [alpha], [OMEGA] are auxiliary variables introduced to take [A.sup.a.sub.[mu]]-field dependence out of the ordered exponential; they are to be integrated out exactly so that dealing with the original time-ordered expressions is guaranteed. Again, this is doable at least in the strong coupling limit of g [much greater than] 1 of a quenching approximation (L[A] = 0).

A 4-pt Green's function illustration can be given. One has basically the expression

[mathematical expression not reproducible], (23)

[mathematical expression not reproducible], (24)

[R.sup.a.sub.i,[mu]](z) = [p.sub.i,[mu]] [integral] d[s.sub.i][[OMEGA].sup.a.sub.i]([s.sub.i])[[delta].sup.4](z - [y.sub.i] + [s.sub.i][p.sub.i]), i = 1,2, (25)

where the dots in the first line of (23) account for the integrand

[mathematical expression not reproducible]. (26)

Now,

[mathematical expression not reproducible], (27)

with

[mathematical expression not reproducible], (28)

and the locality

<x[absolute value of [(gf x [chi]).sup.-1]]y> = [(gf x [chi]).sup.-1](x) [[delta].sup.(4)](x - y). (29)

The 4-pt fermionic Green's function finally reads as

[mathematical expression not reproducible]. (30)

with [Q.sup.a.sub.[mu]](z) being the "currents" given in (24).

(i) This result is obviously gauge-independent, that is, gauge-invariant. It cannot show up in the abelian QED case as long hoped (R. P. Feynman, quoted in [12]). It generalizes to the case of 2n-point fermionic Green's functions [13,14]. When truncated to the YM case, the structure found in [6, 7] is basically reproduced. Eventually, this result lends itself to a (n analytically continued) Random Matrix exact calculation which takes care of the full integration of the [chi]-field dependence and displays the full algebraic dependence of fermionic Green's functions on the [SU.sub.C](3)-Lie algebra invariants [13, 14].

3.2. Effective Locality in the General Case. It is possible to relax any of the approximations used in the "small case" and end up with the property of effective locality. Again this can be illustrated in the simpler case of a fermionic 4-point Green's function:

[mathematical expression not reproducible]. (31)

Gathering Gaussian [A.sup.a.sub.[mu]] dependence of [G.sub.F](1 | A) and [G.sub.F](2 | A),

exp[i/2 [integral] [d.sup.4]z [A.sup.[mu].sub.a](z) [K.sup.ab.sub.[mu]v](z) [A.sup.v.sub.b](z) + i [integral] [d.sup.4]z [Q.sup.[mu].sub.a](z) [A.sup.a.sub.[mu]](z)], (32)

requires 2 extra auxiliary variables; with

[mathematical expression not reproducible], (33)

a new piece of "interaction kernel" reads

[mathematical expression not reproducible] (34)

while "currents" [Q.sup.a.sub.[mu]v](z) get completed into

[mathematical expression not reproducible] (35)

and generalized to a higher number of points of Green's functions in a formally similar way. Restoring the fermionic determinant (i.e., relaxing the quenching approximation), the needed functional operation is now

exp[-i/2 [integral] [delta]/[delta]S x [D.sup.(0).sub.F] x [delta]/[delta]A] x exp[i/2 [integral] A x [bar.K] x A + i [integral] [bar.Q] x A] x exp(L[A]), (36)

followed by the prescription of cancelling the potentials [A.sup.a.sub.[mu]], where

[mathematical expression not reproducible]. (37)

Another differential functional identity is relevant to this operation [11]:

[mathematical expression not reproducible] (38)

where the "cross-linkage" operator exp{[??]} is given by

[mathematical expression not reproducible], (39)

and the limit of [A.sup.a.sub.[mu]] = [A'.sup.a.sub/[mu]] = 0 is to be taken in the end. After cumbersome, still standard, calculations, one gets (up to an irrelevant factor of exp((1/2)Tr ln(-[D.sup.(0).sub.F]))) the functional statement of effective locality as

[mathematical expression not reproducible], (40)

at [mathematical expression not reproducible], that is, locality and gauge independence again, whatever the initial gauge field function one begins with. However the famous duality relation of coupling constants g [right arrow] 1/g is not verified in QCD contrarily to the pure YM case.

This is nontrivial result, the more so if auxiliary field integrations can be carried out exactly, as in the "small case." Now these auxiliary field variables are those related to particular Fradkin's representations, and one may therefore wonder if such a property as effective locality is Fradkin's representation dependent, or not.

3.3. Effective Locality: Even More General. With the functional L[A] being local and fully gauge-invariant, one may consider the case of a fermionic 2-point Green's function generalization to a higher number of points being trivial. One has thus to consider an expression like

[mathematical expression not reproducible], (41)

where, again, the dots in the first line stand for the integrand (26) and, this time, no particular representation is assumed for [G.sub.F][A]. Basically, this is

[mathematical expression not reproducible]. (42)

Up to a global factor of [mathematical expression not reproducible] the core expression, that is, the second line of (41), is

[mathematical expression not reproducible]. (43)

Effective locality is manifest in the first line. In the third line, [G.sub.F][A] is not gauge-independent but acting upon it with the two functional differentiations, followed by the prescription A [right arrow] 0 yielding a manifestly gauge-independent result also. As stated above, it is trivial to check that the same applies to a product of n functionals, [[PI].sup.n.sub.i=1][G.sub.F]([x.sub.i], [y.sub.i] | A), that is, to a 2n-point fermionic Green's function.

One may therefore conclude that while Fradkin's representations are useful to actual calculations and derivations of further remarkable properties, the gist of effective locality does not depend on them. This independence makes of effective locality a property sound enough to support the interpretation proposed in the current article.

Functional integrations (differentiations) reproduce the Feynman graphs perturbative expansions, so that, if not taken literally (analyticity in g on one side, nonanalyticity on the other side), one could propose that the pictorial representation of Figure 1 means effective locality in a symbolic way.

4. Conclusion

Decades of experience with the abelian case of QED have probably made us forget that to calculate observables, it is intrinsically not necessary to select a gauge [15]. To maintain an explicit covariance though, for both historical and practical reasons, one has admitted to break the manifest gauge invariance in QED.

The case of QCD seems to allow one to proceed in a different way, and this is explicitly due to the nonabelian structure of QCD, with its 3 and 4 linear gluonic self-couplings. The result is a generating functional which displays covariant and gauge-independent fermionic Green's functions.

Originally derived on the basis of Fradkin's representations for the closed fermionic loops and background field fermionic propagators, the property of effective locality appears to be more general indeed. The gist of effective locality seems essentially related to the way nonabelian gauge invariance gets realized in the nonperturbative regime of QCD, and this is most easily disclosed by using functional differentiation instead of functional integration.

This situation is new and very different from the abelian case of QED or the perturbative regime of QCD: Up to complications inherent to the nonabelian structure of QCD in effect, gauge invariance follows the same indirect pattern in either cases, Slavnov-Taylor identities playing the role of Ward identities. Reaching the nonperturbative regime of QCD (intense [A.sup.a.sub.[mu]]-fields and/or strong coupling g [much greater than] 1) out of the perturbative sector is now recognized as a dead end because of the Gribov's copy issue which opposes a violent obstruction to this attempt [16, 17].

Such a difficulty does not show up in the effective locality approach, and the fact that gauge invariance in this case is direct may have something to do with the fact that the only QCD states that are outright physical are those of the nonperturbative regime of QCD, that is, states of the hadronic spectrum.

https://doi.org/10.1155/2018/2686507

Conflicts of Interest

The authors declare that there are no conflicts of interest regarding the publication of this paper.

References

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[6] H. Reinhardt, K. Langfeld, and L. V. Smekal, "Phys. Lett," 300, 11, 1993.

[7] H. Reinhardt, "Dual description of QCD," in Proceedings of the conference Quark Confinement and the Hadron Spectrum II, Villa Olmo, Como, Italy, June 26-29, 1996.

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[10] M. B. Halpern, "Phys. Rev," 16, 1798, 1977.

[11] H. M. Fried, Functional Methods and Models in Quantum Field Theory, the MIT Press, Cambridge, MA, USA, 1972.

[12] A. Zee, Quantum Field Theory in a Nutshell, Princeton University Press, 2nd edition, 2010.

[13] T. Grandou, "EPL," Article ID 1650120, 107, 11001, 2014.

[14] H. M. Fried, T. Grandou, and R. Hofmann, "Int. J. of Mod. Phys," 31, Nos. 20 & 21, 1650120, 25 pages, 2016.

[15] A. Maas, "On gauge fixing," in Proceedings of the XXVIII International Symposium on Lattice Field Theory, A. Maas, Ed., Villasimius, Italy, June 2010.

[16] "XIIth Quark Confinement and the Hadron Spectrum," Thessaloniki, Greece, 28 Auust-02 September 2016.

[17] D. Zwanziger, private communication, 1st Winter Workshop in Non-Perturbative Quantum Field Theories, INLN, Valbonne, France, 18-20 January 2010, https://inis.iaea.org/search/search .aspx?orig_q=RN:45045764.

H. M. Fried, (1) T. Grandou (iD), (2) and R. Hofmann (3)

(1) Physics Department, Brown University, Providence, RI02912, USA

(2) Institut de Physique de Nice, UMR CNRS 7010, Universite de Nice-Sophia Antipolis, 1361 route des Lucioles, 06560 Valbonne, France

(3) Institut fur Theoretische Physik, Universitat Heidelberg, Philosophenweg 16, 69120 Heidelberg, Germany

Correspondence should be addressed to T. Grandou; thierry.grandou@inphyni.cnrs.fr

Received 23 August 2017; Accepted 29 March 2018; Published 22 May 2018

Academic Editor: Enrico Lunghi

Caption: Figure 1: Effective Locality pictured in a rather symbolic way in which the sum of all possible QCD interactions between 2 scattering quarks "boils down" to a local contact-type interaction mediated by the structure [(-gf x [chi]).sup.-1](z).
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Title Annotation:Quantum chromodynamics
Author:Fried, H.M.; Grandou, T.; Hofmann, R.
Publication:Advances in High Energy Physics
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Date:Jan 1, 2018
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