Advances in High Energy Physics
Volume 2020 (2020), Article ID 4513698, 12 pages
https://doi.org/10.1155/2020/4513698

Research Article

Solution of the -Deformed Dirac Equation with Vector and Scalar Interactions in the Context of Spin and Pseudospin Symmetries

Claudio F. Farias and Edilberto O. Silva

Departamento de Física, Universidade Federal do Maranhão, 65085-580 São Luís, Maranhão, Brazil

Correspondence should be addressed to Edilberto O. Silva; edilbertoo@gmail.com

Received 27 September 2019; Accepted 9 December 2019; Published 1 February 2020

Academic Editor: Salvatore Mignemi

Copyright © 2020 Claudio F. Farias and Edilberto O. Silva. 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. The publication of this article was funded by SCOAP³.

Abstract.

The deformed Dirac equation invariant under the -Poincaré-Hopf quantum algebra in the context of minimal and scalar couplings under spin and pseudospin symmetry limits is considered. The -deformed Pauli-Dirac Hamiltonian allows us to study effects of quantum deformation in a class of physical systems, such as a Zeeman-like effect, Aharonov-Bohm effect, and an anomalous-like contribution to the electron magnetic moment, between others. In our analysis, we consider the motion of an electron in a uniform magnetic field and interacting with (i) a planar harmonic oscillator and (ii) a linear potential. We verify that the particular choice of a linear potential induces a Coulomb-type term in the equation of motion. Expressions for the energy eigenvalues and wave functions are determined taking into account both symmetry limits. We verify that the energies and wave functions of the particle are modified by the deformation parameter as well as by the element of spin.

1. Introduction

Quantum deformations based on the -Poincaré-Hopf algebra constitute an important branch of research that enables us to address problems in condensed matter and high energy physics through field equations. A pioneer work presenting these equations can be viewed in Ref. [1] (see also Refs. [2–6]), where a new real quantum Poincaré algebra with a standard real structure is obtained by contraction of . The resulting algebra of this contraction is a standard real Hopf algebra that depends on a dimension-full parameter instead of the real deformation parameter . This algebra is defined by the following commutation relations:

where is defined by

with is being the de Sitter curvature and are the -deformed generators for energy and momenta. In the above commutation relations, and represent the spatial rotations and deformed boost generators, respectively. The coalgebra and antipode for the -deformed Poincaré algebra were established in Ref. [7] and have the following representation:

where is the identity operator. The deformed Casimir operators for the -Poincaré algebra have the following representation:

where

With these definitions in hand, we write

The -deformed Dirac operator derived from the above algebra is found to be

and satisfies the following relations:

The square of operator (7) can be written in terms of the invariants and as

or

Since , we can write

In this way, the Dirac equation can be written as

For more details on the derivation of equation (12), see [3], for example. The algebraic structure of the -deformed Poincaré algebra has been widely investigated intensively and has become a theoretical field of increasing interest [5, 6, 8–25]. Through the field equations from the -Poincaré algebra (-Dirac equation [3, 4, 26]), we can study the physical implications of the quantum deformation parameter in relativistic and nonrelativistic quantum systems. In this context, we highlight the study of relativistic Landau levels [22], the Aharonov-Bohm effect taking into account spin effects [21], the Dirac oscillator [27, 28], and the integer quantum Hall effect [29].

When we want to study the relativistic quantum dynamics of particles with spin, it is desirable to consider the presence of external fields, which include the vector and scalar fields. The inclusion of vector and scalar potentials in the Dirac equation reveals interesting properties of symmetries in nuclear theory. The first contributions in this subject revealed the existence of symmetries, which are known in the literature as pseudospin and spin symmetries [30, 31]. Some investigations have been made in this scenario in order to give a meaning to these symmetries. However, it was only in a work by Ginocchio that pseudospin symmetry was revealed. He verified that pseudospin symmetry in nuclei could arise from nucleons moving in a relativistic mean field, which has an attractive scalar and repulsive vector potential nearly equal in magnitude [32] (for a more detailed description, see Ref. [33]). Spin and pseudospin symmetries in the Dirac equation have been studied under different aspects in recent years (see Refs. [34, 35]). Some studies have been developed taking into account the exact spin and pseudospin symmetry limits to study the relativistic dynamics of physical systems interacting with a class of potentials [36–43].

The present work is proposed to investigate the -deformed Dirac equation derived in Ref. [4] in the context of minimal and scalar couplings under spin and pseudospin symmetry limits. The structure of the paper is as follows: In Section 2, we present the -deformed Dirac equation with couplings from which we derive the -deformed Pauli-Dirac equation, by using the usual procedure that consists of squaring the -deformed Dirac equation. In Section 3, we consider the equation of Pauli and establish the spin and pseudospin symmetry limits. As an application, we consider the particle interacting with a uniform magnetic field in the -direction in two different physical situations: (i) particle interacting with a harmonic oscillator and (ii) particle interacting with a linear potential. We obtain expressions for the energy eigenvalues and wave functions in both limits. In Section 4, we present our comments and conclusions.

2. The -Deformed Dirac Equation with Couplings

In this section, we introduce the minimal and scalar substitutions into -deformed Dirac equation (12). Before doing this, let us write it in a more convenient way to be treated. This can be accomplished by multiplying the left of equation (12) by and retaining terms up to . The resulting equation is found to be [3, 4]

Deformed Dirac equation (13) is invariant under the -deformed Poincaré quantum algebra. Manipulating this equation and using the properties of the Dirac matrices and then rearranging the terms, it is possible to write it in the Hamiltonian form, , where is the -deformed Dirac Hamiltonian and are the energy eigenvalues. After identifying , with , we can iterate equation (13). This development yields to

where we have discarded the terms of order equal and superior to on the iterative replacements of the energy . The interactions can be introduced through the following prescriptions [44]:

where is the electric potential, is the vector potential, and is the scalar potential. It is known from relativistic quantum mechanics that for vector coupling the potential couples to the charge (which is different for particles and antiparticles) while for scalar coupling the potential couples to the mass (which is equal for both particles and antiparticles).

As mentioned in Ref. [4], the couplings ((15), (16), and (17)) are quite satisfactory from the point of view of the -Poincaré-Hopf algebra. Indeed, there are no operator ordering problems after the gauging that would require symmetrization in equation (13). Using these couplings, we obtain the following expression:

Since we are interested in planar dynamics, i.e., when both and as well as the third directions of the fields involved are zero, we choose the following representation for the gamma matrices in terms of the Pauli’s matrices [45]:

where parameter , which has a value of twice the spin value, can be introduced to characterizing the two spin states, with for spin up and for spin down. The matrices satisfy the properties

Using the representation and the properties of the Pauli’s matrices above, the -deformed Dirac equation including the interactions can be written as

where the magnetic field emerges when we use the relation

Let us now determine the Dirac equation in its quadratic form. This can be accomplished by applying the matrix operator [46, 47]

in equation (21). In this procedure, we follow a similar algebra and the same mathematical properties of the parameters and variables involved on the deduction of equation (21). The result is the -deformed Dirac-Pauli equation

It can be easily verified in equation (24) that after considering , the resulting equation is the one well known in the literature (see, for example, Ref. [48]). In order to apply equation (24) to a given physical system, we need to choose a representation for the vector potential and the scalar potentials and . For some particular choices of these quantities, we can study the physical implications of quantum deformation on the properties of various physical systems of interest.

For the field configuration, we consider a constant magnetic field along the -direction (in cylindrical coordinates), , which is obtained from the vector potential (in the Landau gauge) [49],

In this configuration, equation (24) reads

with

where the matrices (19) are now given in cylindrical coordinates, , , with [48]

We will attribute expressions to functions and in equation (26) in the next section, when we treat the analysis of spin and pseudospin symmetries. We will argue after that only some particular choices for these functions will lead to a differential equation that admits an exact solution.

3. Symmetry Limits

To implement the spin and pseudospin symmetry limits, we make in equation (26) the requirement that , where the plus (minus) signal refers to spin (pseudospin) symmetry, respectively [32]. Next, by using , the first and second lines in equation (26) can be written in a simple form, which allows us to solve them separately. Furthermore, as mentioned above, we need to choose a representation for the radial function . We give a representation in terms of cylindrically symmetric scalar potentials which lead to results well-known in the literature.

3.1. Particle Interacting with a Harmonic Oscillator

It is well known that the harmonic oscillator can be used to describe a large number of physical systems. The interest in this issue appears in physical systems at an atomic scale and extends to high energy physics. It appears, for instance, as the interaction between atoms in the elastic crystal [50–52], as the effective potential acting on electrons moving in a uniform magnetic field (Landau levels) [49, 53–57] and in the quantization of the electromagnetic field [58]. The potential of the harmonic oscillator is included into equation (26) by making , where is a constant. One can check that the spin symmetry is sufficient to decouple the radial equation that comes from the upper spinor component while the pseudospin symmetry decouples the radial equation that comes from the lower component of the spinor. Thus, by adopting solutions of the form

we arrive at radial equations

where , , , , , , and . It is convenient to write equation (30) in a known canonical form. This can be accomplished using as

where , which leads to the equation

Equation (32) is of the confluent hypergeometric equation type, and its solution is given in terms of the Kummer functions. In this manner, the general solution for equation (32) is given by [59]

where are the Kummer functions. In particular, when , with , the function becomes a polynomial in of degree not exceeding . From this condition, we extract the energies for the spin and pseudospin symmetry limits, given, respectively, by

Equations (34) and (35) are, respectively, the particle and antiparticle energies in the context of quantum deformation, and they can be read as a relativistic generalization of the Landau levels. It must be emphasized that, since and are positive, the quantum deformation affects the separation of the energy levels of the system. This feature, however, should not depend on the value of the spin projection parameter . Figure 1 shows energy profile (34) as a function of the frequency for some values of the quantum number . In Figure 1(a), we plotted for and in Figure 1(b) for . In this analysis as well as for the others, we use [18, 29]. For this value, the effects of quantum deformation become more evident. We clearly see that both particle and antiparticle belong to the same energy spectrum. However, in Figure 1(b), we find that the antiparticle energy is not defined in the frequency ranges (for ) and (for ). These same characteristics are also present in the energy profile of equation (35) as shown in Figure 2. However, in Figure 2(b), the energies are not defined in the frequency ranges (for ), (for ), and (for ). The appearance of such regions characterizing the absence of energy eigenvalues is due to the quantum deformation effects present in the model. On the other hand, when we compare the energy (34) (spin symmetry case) with the energy (7) of Ref. [28], we observe the absence of the interaction term between the Dirac oscillator and the angular momentum. Here, the frequency comes from the gauge field (25), which couples with the spin of the particle. Although these spectra are similar, physically, they are different. In fact, when , we obtain the energy eigenvalues of Ref. [48] (after removing the magnetic flux parameter), which shows the consistency of the model in question. In particular, when and are null, we obtain

which are the usual relativistic Landau levels with the inclusion of the element of spin.

(a)

(b)

Figure 1: Illustration of the energy eigenvalues in the spin symmetry limit (equation (34)) as a function of the parameter for (a) and (b) . We use units such as , , , and an upper bound .

(a)

(b)

Figure 2: Illustration of the energy eigenvalues in the pseudospin symmetry limit (Eq. (35)) as a function of the parameter for (a) and (b) . We use units such as , , and an upper bound .

3.2. Particle Interacting with a Linear Potential

Let us consider the case where the particle interacts with a linear potential, . As discussed above, linear interactions are included in the relativistic motion equations through the quadripotential . In the case of the Dirac equation, depending on the configuration of external potentials involved, it can be solved exactly. An example of an exactly soluble model described by a linear interaction in relativistic quantum mechanics is the Dirac oscillator [60]. It is known that the Hamiltonian of the Dirac oscillator describes the interaction of a neutral particle with an electric field via an anomalous magnetic coupling [61]. In the context of confinement of quarks in mesons and baryons, it is well established that electrostatic linear potentials lead to the occurrence of the Klein paradox and particles cannot be confined [62]. To establish such confinement, we must invoke the scalar substitution (17). In this case, we make (where is a constant) in equation (26) to the limits of spin and pseudospin symmetries and proceed as before. The resulting equation is given by

with , , , , , , , and . In equation (37), the signs refer to spin and pseudospin symmetries, respectively. By performing the variable change, , equation (37) assumes the form

where we have defined the parameters , , and . Note that the choice induces a Coulomb-like interaction in the resulting deformed sector of the eigenvalue equation. The origin of this Coulomb potential is due purely to the quantum deformation and boundary symmetries involved.

Equation (38) is of the Heun equation type, which is a homogeneous, linear, second-order, differential equation defined in the complex plane [63]. This equation can be put into its canonical form using the solution

where satisfies the biconfluent Heun differential equation

with , , , and . Equation (40) has a regular singularity at and an irregular singularity at of rank . Usually, the solution of this equation is given in terms of two linearly independent solutions as

where (assuming that is not a negative integer)

are the Heun functions. After the insertion of this solution into equation (40), we find ()

where

From the recursion relation (45), the function becomes a polynomial of degree if and only if the two following conditions are imposed [63]:

where is a positive integer. In this case, the coefficient in the series expansion is a polynomial of degree in . When is a root of this polynomial, the and subsequent coefficients cancel and the series truncates, resulting in a polynomial form of degree for . From condition (47), we extract the energies at the spin and pseudosymmetry limits, given, respectively, by

The energy of a physical system must be a function involving all the parameters present in the equation of motion. In equation (49), the parameter is absent. However, it can be restored using condition (48) from which we obtain a relation between such parameter and the frequency of the system. For each value of fixed, we have a self-energy and its corresponding wave function. Let us consider solution (42) up to second order in of the expansion,

If we truncate the series in a term of order , the resulting finite series is related, via solution (39), to the energy level . Thus, the physical quantity that we can associate most closely with the series (50) truncated in the term is the energy of the particle with the wave function (39). In fact, it is necessary that the series (50) becomes an -degree polynomial for the system to admit bound states. Thus, by using relation (45) and equations (43) and (44), the coefficient above can be determined. If we want to truncate solution (50) in , we must impose that through condition (48); when we truncate in , we make , and so on. For each of these cases, we can establish appropriate constraints between conditions (47) and (48). Since equation (49) is of the relativistic Landau level type, we prefer to fix the frequency in order to obtain an expression for the energies corresponding to each value of [41, 64–70]. Since it is done for both spin and pseudospin symmetries, we also label the frequency as , with the subscript characterizing the values to be fixed. After obtaining and replacing them in equation (49), we will have expressions for the energies involving the quantities , , , and , which contains the coupling constant , the mass of the particle , and the quantum angular momentum number . Thus, for , it means that we are investigating the particular solution for . In this case, from equation (44), we have

where . Solving (51) for , we get the relations

Proceeding in a similar way to , we find the following third-degree polynomial in ():

with

where and . Equation (53) has only one real root. For each specific frequency, and , we can determine the energies and by the following expressions:

where is given by

with

and the requirement that . Such energies represent the first two energy levels of the system. For simplicity, we perform a numerical analysis only for the case . In this way, by studying equation (55), we find that for and , the energy of the particle is infinitely degenerate, with respective eigenvalues and , whereas for , only one of the roots is infinitely degenerate with energy (Figure 3(a)). On the other hand, when we analyze equation (55) for , we verify that the energy spectrum is defined only for , and one of the roots is infinitely degenerate with eigenvalue (Figure 3(b)). These characteristics are also present in the energies from equation (56). For , the energies are defined only for and one of the roots is infinitely degenerate, with eigenvalue (Figure 4(a)). For and , there is an infinitely degenerate root with eigenvalue while for both roots are infinitely degenerate with respective energies and (Figure 4(b)).

(a)

(b)

Figure 3: Illustration of the energy eigenvalues in the spin symmetry limit (equation (55)) as a function of the parameter for (a) and (b) . We use units such as , , , and .

(a)

(b)

Figure 4: Illustration of the energy eigenvalues in the pseudospin symmetry limit (equation (56)) as a function of the parameter for (a) and (b) . We use units such as , , , and .

To determine the energies corresponding to , we must make use of the above recipe. However, as we can see from equation (53), the polynomials of degree resulting from condition (48), in general, not all roots are physically acceptable. In the absence of deformation, the resulting equation describes the motion of an electron subject to interactions (15), (16), and (17). In the literature, models in this context can be found. With the presence of these interactions in the Dirac equation, the wave function depends on several parameters. Thus, if we consider a null deformation, a direct comparison with particular cases in the literature is not immediate. The reader can see some examples in Refs. [41, 71–73].

4. Conclusions

We have studied the relativistic quantum dynamics of a spin charged particle with minimal and scalar couplings in the quantum deformed framework generated by the -Poincaré-Hopf algebra. The problem has been formulated using the -deformed Dirac equation in two dimensions. The -deformed Pauli equation was derived to study the dynamics of the system taking into account the spin and pseudospin symmetry limits. For the -deformed Dirac-Pauli equation obtained (equation (26)), we have argued that only particular choices of radial function lead to exactly solvable differential equations. We have considered the case where the particle interacts with a uniform magnetic field, a planar harmonic oscillator, and a linear potential. We have verified that the linear potential leads to a Coulomb-type term in the -deformed sector of the radial equation. The resulting equation obtained is a Heun-type differential equation. Analytical solutions for both spin and pseudospin symmetry limits enabled us to obtain expressions for the energy eigenvalues (through the use of equations (47) and (48)) and wave functions. Because of the limitations imposed by condition (48), we have derived expressions for the energies corresponding only to (equations (55) and (56)) and (equations (57) and (58)). We have shown that the energy eigenvalues and wave functions are modified by both the spin element and the deformation parameter . We believe that future experiments may provide some estimate on the magnitude of the deformation parameter within the context of the model studied.

Data Availability

We did not use any data in this paper.

Conflicts of Interest

The authors declare that there is no conflict of interests regarding the publication of this paper.

Acknowledgments

EOS acknowledges funding from Conselho Nacional de Desenvolvimento Científico e Tecnológico (CNPq) (Grant Nos. 427214/2016-5 and 303774/2016-9) and Fundação de Amparo à Pesquisa e ao Desenvolvimento Científico e Tecnológico do Maranhão (FAPEMA) (Grant Nos. 01852/14 and 01202/16).

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