Advances in Mathematical Physics

Volume 2011 (2011), Article ID 652126, 12 pages

http://dx.doi.org/10.1155/2011/652126

## Gauge and Lorentz Transformation Placed on the Same Foundation

^{1}Loodus- ja Tehnoloogiateaduskond, Füüsika Instituut, Tartu Ülikool, Riia 142, 51014 Tartu, Estonia^{2}Institut für Physik, Johannes-Gutenberg-Universität, Staudinger Weg 7, 55099 Mainz, Germany

Received 25 March 2011; Accepted 14 April 2011

Academic Editor: H. Neidhardt

Copyright © 2011 Rein Saar et al. This is an open access article distributed under the Creative Commons Attribution License, which permits unrestricted use, distribution, and reproduction in any medium, provided the original work is properly cited.

#### Abstract

We show that a “dynamical” interaction for arbitrary spin can be constructed in a straightforward way if gauge and Lorentz transformations are placed on the same foundation. As Lorentz transformations act on space-time coordinates, gauge transformations are applied to the gauge field. Placing these two transformations on the same ground means that all quantized field like spin-1/2 and spin-3/2 spinors are functions not only of the coordinates but also of the gauge field components. As a consequence, on this stage the (electromagnetic) gauge field has to be considered as classical field. Therefore, standard quantum field theory cannot be applied. Despite this inconvenience, such a common ground is consistent with an old dream of physicists almost a century ago. Our approach, therefore, indicates a straightforward way to realize this dream.

#### 1. Introduction

After the formulation of general relativity which explained fources on a geometric ground, physicists and mathematicians tried to incorporate the electromagnetic interaction into this geometric picture. Weyl claimed that the action integral of general relativity is invariant not only under space-time Lorentz transformations but also under the gauge transformation, if this is incorporated consistently [1]. However, the theories at that time were not ready to incorporate this view. Nowadays, we see more clearly that all physical variables (like position, momentum, etc.), quantum wave functions, and fields transform as finite-dimensional representations of the Lorentz group. The reason is that interactions between fundamental particles (as irreducible representations of the Poincaré group) are most conveniently formulated in terms of field operators (i.e., finite-dimensional representations of the Lorentz group) if the general requirements like covariance, causality, and so forth are to be incorporated in a consistent way. The relation between these two groups and their representations is given by the Lorentz-Poincaré connection [2]. In this paper we show that if gauge transformation is put on the same foundation, the resulting nonminimal “dynamical” interaction obeys all necessary symmetries which for higher spins are broken if the interaction is introduced by the usual minimal coupling.

In Section 2 we explain details of the Poincaré group which are necessary in the following. In Section 3 we deal with linear wave equations as objects to the Lorentz transformation. In Section 4 we introduce the external electromagnetic field by a nonsingular transformation. In Section 5 we specify the nonlinear transformation by the claim of gauge invariance of the Poincaré algebra. Finally, in Section 6 we give our conclusions.

#### 2. The Poincaré Group

Relativistic field theories are based on the invariance under the Poincaré group (known also as inhomogeneous Lorentz group [2–11]). This group is obtained by combining Lorentz transformations and space-time translations , The group’s composition law generates the semidirect structure of , where is the abelian group of space-time translations (i.e., the additive group ) and is the proper orthochronous Lorentz group acting on the Minkowski space with metric The condition of the metric to be invariant under Lorentz transformations takes the form Under the Lorentz transformation the transformation of the covariant functions according to a representation of the Lorentz group [3–16] is determined by the commutative diagram (2.5) That is, The map is a finite-dimensional representation of . If we parametrize the element by where the Lorentz generators are given by and are six independent parameters, the parametrization of reads The Lorentz group is noncompact. As a consequence, all unitary representations are infinite dimensional. In order to avoid this, we introduce the concept of -unitarity (see, e.g., [9] and references therein). A finite representation is called -unitary if there exists a nonsingular Hermitian matrix so that Notice that an -unitary metric is always indefinite, so that the inner product generated by is sesquilinear sharing the hermiticity condition . The most famous case of -unitarity is given in the Dirac theory of spin-1/2 particles where .

For an operator [17, 18] acting on the -space of covariant functions (we have to impose the action on covariant functions because in case of higher spins the relations between operators we obtain are valid only as weak conditions) the transformation in (2.6) is a covariant transformation if the diagram(2.10)

is commutative, that is, Using (2.6) we obtain Notice that the covariance of the transformation embodies only the property of equivalence of reference systems. The covariant operator is invariant under transformation (2.6) if in addition . As a consequence we obtain the commutative diagram (2.13) or which means on the -space. The invariance is a symmetry of the physical system and implies the conservation of currents. In particular, the symmetry transformations leave the equations of motion form-invariant.

While the Lorentz transformation changes the wave function itself as well as the argument of this function (cf. (2.6)), the proper Lorentz transformation causes a change of the wave function only. On the ground of infinitesimal transformations, this change is performed by the substantial variation. Starting from an arbitrary infinitesimal coordinate transformation , the substantial variation is given by [13] where , . The corresponding finite proper Lorentz transformation can be written as and the multiplicative structure of the group generates the adjoint action Due to (2.9) the generators fulfill . They depend on the spin of the field but not on the coordinates . Therefore, we have . If a generic element of the translation group is written as the commutator relations of the Lie algebra are given by The Casimir operators of the algebra are and , where is the Pauli-Lubanski pseudovector, . In coordinate representation we have , and the finite Poincaré transformation has the form This relation constitutes the Lorentz–Poincaré connection [2]. While the representation generally generates a reducible representation of , the spectra of the Casimir operators and determine the mass and spin content of the system.

#### 3. The Wave Equations

As an operator in the above sense we consider the operator of the wave equation. The Dirac-type wave equation we will consider has the form where is an -component function, , and are matrices independent of . Following Bhabha's conception [19], it is “…logical to assume that the fundamental equations of the elementary particles must be first-order equations of the form (3.1) and that all properties of the particles must be derivable from these without the use of any further subsidiary conditions.”

The principle of relativity states that a change of the reference frame cannot have implications for the motion of the system. This means that (3.1) is invariant under Lorentz transformations. Equivalently, the Lorentz symmetry of the system means the covariance and form-invariance of (3.1) under the transformation in (2.6), that is, the transformed wave equation is equivalent to the old one. Therefore, we require that every solution of the transformed equation can be obtained as Lorentz transformation of the solution of (3.1) in the original system and that the solutions in the original and transformed systems are in one-to-one correspondence. The explicit form of the covariance follows from (2.11), and leads to the explicit Lorentz transformations The Lorentz invariance is given by the substitution or The difference of the original and transformed wave equation is given by the wave equation where the wave function is replaced by the substantial variation , . As a consequence we obtain or An excellent discussion of such matrices can be found in [13, 19–23]. The hermiticity of the representation in (2.9) implies the hermiticity of (3.1). Including a still unspecified Hermitian matrix the hermiticity condition reads or Writing , one obtains the adjoint equation

#### 4. Introduction of the External Field

It may be reasonable to introduce an external field directly into the Poincaré algebra which can be applied to classically understand the elementary particle. To do so one has to transform the generators of the Poincaré group to be dependent on the external field in such a way that the new, field-dependent generators obey the commutation relations (2.19). As it was proposed by Charkrabarti [24] and Beers and Nickle [25], the simplest way to build such a field-dependent algebra is to introduce the external field by a nonsingular transformation In case of a particular external electromagnetic field , the external field can be introduced by using an evolution operator , called the “dynamical” representation [26, 27]. By analogy with the free-particle case one can realize this representation on the solution space of relativistically invariant equations. Expressing the operators explicitly in terms of free-field operators, one obtains the “dynamical” interaction. Applying, for instance, the operator to (3.1) one obtains where and (here and in the following we will skip the argument for and the argument for ). Having introduced the external gauge field , we introduce gauge covariance on the same foundation as Lorentz covariance in (2.6), that is, by claiming that the diagram (4.4) is commutative, that is, According to (2.13), the “dynamical” interaction is gauge invariant under the gauge transformation if the diagram (4.6)

is commutative, that is, Together with (4.5) we obtain or on the -space. Note that up to now we have not specified the explicit shape of the finite-dimensional representation of the gauge group.

#### 5. Specifying by Gauge Invariance

At this point we specify by two claims. Due to gauge symmetry as a fundamental principle the dynamical transformation has to be compatible with the gauge transformation. Therefore, we first claim the gauge invariance in (4.8) not only for the operator but for the whole dynamical Poincaré algebra , By using (4.1) and multiplying by from the right we obtain This means that the first claim is fulfilled if On the other hand, with (4.3) and (4.5) we obtain and, therefore, on the -space. To summarize, by the first claim the gauge symmetry determines the gauge properties of and, therefore, of the interacting field .

The second claim is that the dynamical transformation operator should be of Lorentz type, that is, for the generators of the Poincaré algebra one has which is a local extension of (2.17). is the local Lorentz transformation generated by the external field and obeying If such a local Lorentz transformation exists, the problem is solved. Therefore, in the following we make the attempt to find explicit realizations of the local Lorentz transformation . It is hard to find the Lorentz transformation in general. However, as first shown by Taub [28], in the case of a plane-wave field we obtain where is the electric charge of the particle and . The plane-wave field , is characterized by its lightlike propagation vector , , and its polarization vector such that and . The operator commutes with any other and has a special role in the theory. For particles with nonzero mass one has . Therefore, for the plane wave the differential operator is local and well defined for the plane-wave solution of the Klein-Gordon equation. In all other cases, is assumed to exist.

Note that the plane-wave solution of the Dirac equation was found more than 70 years ago by Wolkow [29] and extended later on to a field of two beams of electromagnetic radiation [30, 31]. However, these approaches did not make use of the nonsingular transformation . The realization of can be achieved by the nonsingular transformation , where It has to be mentioned that the evolution operator may be chosen to be -unitary according to the representation in (2.9), that is, Considering the nonsingular transformation of Dirac-type wave equation with the help of (5.8) the “dynamical” counterparts to the operator can be calculated to be , () while the “dynamical” counterpart to is given by , In terms of and we have However, expressed in terms of and , we obtain where . This interaction is nonminimal. However, as we have shown before, it is determined completely by the claim of gauge invariance.

Note that due to the antimutation of the -matrices, in the spin-1/2 case the dynamical interaction in (5.15) reduces to the minimal coupling. However, in order to obtain the correct values of the gyromagnetic factor, in some cases the (phenomenological) Pauli term has to be added by hand to the minimal coupling of the Dirac equation (see also [32, page 109]). In case of plane waves the exact solution of this (supplemented) Dirac equation as given by Charkrabarti [24] obeys the same gauge invariance condition . This property is found also in the book by Fried [33].

Finally, as a consequence of the explicit form (5.8), the associated transformation of the evolution operator under the local gauge transformation for the plane wave field, becomes As an example of higher spin, the spin-3/2 case is considered in detail in [34]. As it turns out, the Rarita-Schwinger spin-3/2 equation on the presence of a “dynamical” interaction is algebraically consistent and causal.

#### 6. Conclusions

As a consequence of gauge invariance and Lorentz type of we obtain (1)the invariance of the wave function under gauge transformations, that is, , (2)the explicit shape of in (4.5), that is, , (3)the invariance of under gauge transformations from (4.7) and that is, on the -space, (4)the “dynamical” interaction for any spin as given by being nonminimal but completely determined by gauge invariance, thereby causing Poincaré symmetry,(5)as a consequence of (5.12), the gyromagnetic factor in the presence of a “dynamical” interaction as being for any spin [27].

Let us close again with Weyl In [1] he honestly confessed: *“Die entscheidenden Folgerungen in dieser Hinsicht verschanzen sich aber noch hinter einem Wall mathematischer Schwierigkeiten, den ich bislang nicht zu durchbrechen vermag.”* (“*However, the crucial consequences in this respect entrench oneself still behind a bank of mathematical difficulties which up to now I am not able to penetrate.”*) We hope that our work breaks a small bay into this mathematical bank.

#### Acknowledgments

The work is supported by the Estonian target financed Project no. 0180056s09 and by the Estonian Science Foundation under grant no. 8769. S. Groote acknowledges support by the Deutsche Forschungsgemeinschaft (DFG) under Grant 436 EST 17/1/06.

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