Relativistic fermion on a ring: energy spectrum and persistent current.
The existence of a persistent current in a normal metallic ring threaded by a magnetic flux has stimulated a large number of studies in last few decades [1-10]. The current is periodic in flux like the current in a superconducting ring 11-14]. Due to the recent advances in fabrication techniques, it has become possible to observe this current experimentally [15-18] in mesoscopic systems. Such current is also found in carbon nanotube rings [19-21]. In these carbon based structures, electrons behave as massless Dirac particles and they require a relativistic description. Although there have been significant amount of work on the energy levels and persistent current of relativistic fermion regarding graphene [22-32], topological insulator  and for neutrino billiards  and Dirac electron , there is still lack of a complete description of persistent current for relativistic fermions and its variation with particle mass. Besides, it is well known that superconducting as well as mesoscopic rings are perfect diamagnets, but carbon nanotube tori  are found to possess a positive susceptibility. There is no vivid discussion on how the transition occurs.
In this paper, we have studied the nature of energy and persistent current spectra for a relativistic particle on a one-dimensional ring. We describe the scenario for all the mass regime and explain the massless case as well. For heavy fermions, our findings are in good agreement with the non-relativistic behaviour . Interesting features are revealed as we move towards the relativistic regime, that is, for low mass. The flux dependence of the current becomes more and more nonlinear as we decrease the mass. For a particular ring radius, we find the existence of a critical mass at which the current becomes constant in flux. The value of this current is the same as the current produced by a massless particle and it appears to be the lower cutoff for current as we further decrease the mass. This nature is prominent for massless particle as well. We further study the nature of the total current and find that it shows periodic plateaus. It becomes a multiple step function at critical mass and becomes discrete below that mass. The same periodicity is also observed in the susceptibility. More interestingly, we find that its amplitude changes from negative to positive value as we decrease the mass. This is further clarified by studying the behaviour of the susceptibility with respect to mass at a particular flux value. Same behaviour is observed if we keep the mass fixed and treat the ring radius as parameter.
The organisation of the paper is as follows. In Section 2, we give a brief description about the Dirac equation and its solution on a circle. Then we obtain the energy spectrum in presence of an Aharonov-Bohm flux. We derive the resulting persistent current in Section 3 and show its behaviour for different mass range specially for a massless fermion. In Section 4, we discuss the behaviour of total current and in Section 5, the nature of susceptibility is discussed. Section 6 contains a proposed experiment to verify the result. The discussion is kept in Section 7.
2. Relativistic Particle on a One-Dimensional Ring
We start with a very brief description of Dirac equation on a circle. Then we will derive its solution in presence of an Aharonov-Bohm flux and obtain the energy spectrum.
Dirac equation in two dimensions is given by 
[MATHEMATICAL EXPRESSION NOT REPRODUCIBLE IN ASCII], (1)
where [psi] = [([[zeta].sub.1], [[zeta].sub.2]).sup.T] is a two component spinor and [MATHEMATICAL EXPRESSION NOT REPRODUCIBLE IN ASCII] are Pauli matrices. Due to the symmetry of the problem, it would be easier to work with polar coordinate (x = R cos([phi]), and y = R sin([phi]): R is the ring radius) in which the Dirac Hamiltonian becomes
[MATHEMATICAL EXPRESSION NOT REPRODUCIBLE IN ASCII], (2)
[MATHEMATICAL EXPRESSION NOT REPRODUCIBLE IN ASCII]. (3)
Note that (2) is similar to the Hamiltonian used in . They have used 4 x 4 Dirac matrices whereas we use here 2 x 2 representation which finally leads to the same dispersion relation. It is worth mentioning that one should be careful while deriving a Dirac Hamiltonian for a lower dimension. Remember that number of Dirac matrices required for a d + 1 (spacetime) dimensional space is d + 1 and they must satisfy the corresponding Dirac algebra. One can start from a two-dimensional Dirac Hamiltonian and replace the radial variable dependent terms with their expectation values considering a vanishing width of the radial wave function [24, 25, 38]. In this way, although it is possible to reduce a spatial dimension, the resulting Hamiltonian may still need three Dirac matrices (One can check that by using <r> = 0 and <[partial derivative]/[partial derivative]r> = -1/2R  in a two-dimensional polar Dirac equation.) and that will be a contradiction about the dimensionality of the system. A better way would be to use the constraint relations and obtain the Hamiltonian in terms of the generalised coordinate which we have done here. The Hamiltonian (2) we derive here involves only two Dirac matrices ([[sigma].sub.[phi]], [[sigma].sub.3]) which is in tone with the one dimensionality of the system.
Now let us consider a perpendicular magnetic field piercing the ring (Figure 1). A suitable choice for vector potential (under symmetric gauge) is
[MATHEMATICAL EXPRESSION NOT REPRODUCIBLE IN ASCII], (4)
where [PHI] is the total flux passing through the ring.
The energy of the system is given by 
[E.sub.l] = [square root of ([m.sup.2][c.sup.4] + [(c[??]/R).sup.2] (l + ([PHI]/[[PHI].sub.0])) (l + ([PHI]/[[PHI].sub.0]) - 1), (5)
where I = 0, [+ or -] 1, [+ or -] 2, ... and [[PHI].sub.0] = ch/e is the flux quanta.
One can see (Figure 2) that the energy varies parabolically with respect to [PHI] and has periodicity of [[PHI].sub.0]. This is similar to the case of a nonrelativistic particle . The only difference is the fact that the minima of the energy are at half integral multiple of [[PHI].sub.0]. This shift by [[PHI].sub.0]/2 appears due to relativistic correction .
3. Persistent Current for a Dirac Particle
We will now discuss the nature of energy spectrum and resulting persistent current for different mass regime.
Persistent current is the perpetual current flowing in a superconducting or normal metallic ring in the presence of a Aharonov-Bohm flux. It is given by the flux derivative of the energy [3, 14]
[I.sub.l] = -c [partial derivative][E.sub.l]/[partial derivative][PHI]. (6)
For a Dirac particle on a one-dimensional ring whose energy is given by (5), the persistent current is
[I.sub.l] = - e[??]/2[pi]m[R.sup.2] l + ([PHI]/[[PHI].sub.0]) - (1/2)/[square root of (1 + [([??]/mcR).sup.2](l + ([PHI]/[[PHI].sub.0]))(l + ([PHI]/[[PHI].sub.0]) - 1))]. (7)
One can regain the nonrelativistic result for m [right arrow] [infinity]. At this limit the, current is given by
[I.sub.l][|.sub.m [right arrow] [infinity]] = -e[??]/2[pi]m[R.sup.2] (l + [PHI]/[[PHI].sub.0] - 1/2). (8)
The expression looks similar to the nonrelativistic current . The only difference is that like the energy spectrum, it also undergoes a shift by [[PHI].sub.0]/2 with respect to the flux. However the behaviour of current at relativistic regime (m [right arrow] 0) is rather complicated. To have an idea about the flux dependence of the current, we will study the single particle susceptibility [[OMEGA].sub.l]([kappa], [PHI]) defined as
[MATHEMATICAL EXPRESSION NOT REPRODUCIBLE IN ASCII], (9)
[I.sub.0] = e[??]/2[pi]m[R.sup.2], (10)
[kappa] = [([??]/mcR).sup.2]. (11)
Now we will discuss the behaviour of [[OMEGA].sub.l]([PHI], [kappa]) for different ranges of [PHI] and [kappa]. Consider the following
(a) [kappa] [right arrow] 0: [[OMEGA].sub.l]([PHI], [kappa]) [right arrow] -[I.sub.0]/[[PHI].sub.0] which is negative, constant and independent of l. Hence the current will vary linearly with flux for all I values. This is actually the nonrelativistic (m [right arrow] [infinity]) limit.
(b) [kappa] = 4: [[OMEGA].sub.l]([PHI], k) = 0; that is, the current will not depend on the flux. We call the corresponding mass to be the critical mass for radius R, given by
[m.sup.R.sub.cri] = [??]/2cR. (12)
The constant current is given by
[I.sub.sat] = [I.sub.0]/[kappa] = -ec/2[pi]R. (13)
This is actually current generated by a massless particle with charge e.
(c) [kappa] > 4: this is the low mass limit. At [PHI] [right arrow] [infinity] limit, the current becomes constant, given by (13). For [kappa] > 4, [[OMEGA].sub.l]([OMEGA], [kappa]) blows up at
[PHI]/[[PHI].sub.0][|.sub.div] = (1/2 - l) [+ or -] 1/2 [square root of (1 - (4/[kappa]))], (14)
which are actually the roots of the denominator of (9). The divergence in [[OMEGA].sub.l]([PHI], k) suggests discontinuity in current. For [kappa] [right arrow] [infinity] (m _ 0, i.e., massless limit), the divergence occurs at [PHI]/[[PHI].sub.0] = -l and [PHI]/[[PHI].sub.0] = -l + 1. Note that within these two diverging limits, the energy becomes a imaginary quantity and hence the corresponding states will be decaying states. Appearance of such nonhermiticity of Dirac Hamiltonian is well known in curved space . In our case, it is an artefact of the geometry of the system.
The nature of energy and current in these three k region is shown in Figure 4. Figures 2 and 3 show the energy and current spectra for [kappa] = 0.01 (R = 10[r.sub.e], m = 1[m.sub.e]) which are an example for [kappa] = 0 regime.
One can also observe the same nature of current by keeping m fixed and varying R as a parameter. In that case, there would be a critical radius given by
[R.sup.m.sub.cri] = [??]/2mc, (15)
at which, the currentbecomes constant. This is actually half of the reduced Compton wavelength of the particle. However by tuning the radius, it is not possible study the phenomena for massless particles.
3.1. Persistent Current for a Massless Dirac Particle. As a special case, we will discuss here the nature of persistent current caused by a massless particle. The energy of such particle can be obtained by putting m = 0 in (5) and is given by
[E.sup.0.sub.l] = (c[??]/R) [square root of ((l + ([PHI]/[[PHI].sub.0]))(l + ([PHI]/[[PHI].sub.0]) - 1))]. (16)
Corresponding persistent current by definition (6) is
[I.sup.0.sub.l] = -ec/2[pi]R l + ([PHI]/[[PHI].sub.0]) - (1/2)/[square root of (l + ([PHI]/[[PHI].sub.0]))(l + ([PHI]/[[PHI].sub.0]) - 1). (17)
The variation of [E.sup.0.sub.l] and [I.sup.0.sub.l] with flux is shown in Figure 5.
From the denominator of (17), one can readily see that for [PHI]/[[PHI].sub.0] = -l and [PHI]/[[PHI].sub.0] = -l + 1, the current diverges. This is something that does not happen for a nonrelativistic particle. At asymptotic region ([PHI]/[[PHI].sub.0] [right arrow] [infinity]), the current becomes constant (Figure 5) and is given by (13) which is the current produced by a massless particle with charge e circling in a ring of radius R.
4. Total Current for Odd and Even Number of Particles
From (17), one can understand that an exact analytic expression for total current is not possible for our case (For an approximate result at large mass limit see ). We consider 100 particles in a ring with radius R = 10re and numerically evaluate the total current for different m values. While doing so, we consider only Pauli's exclusion principle and neglect any other kinds of interaction among the particles. The result for both even and odd number of particles is shown in Figure 6.
From Figure 6, we see that for large mass, total current varies linearly with flux (Figure 6(a)). This is consistent with the nonrelativistic result. As we decrease the mass, relativistic effects start dominating and the current starts showing nonlinear behaviour (Figure 6(b)). This is manifested by the periodic appearance of flat regions in Figure 6(b). Atm = [m.sup.R.sub.cri] (12) ([kappa] = 4) total current becomes a multiple step function of flux (Figure 6(c)), the step heights being integral multiple of [I.sub.sat] (13) and each step being 2[I.sub.sat] high. As we further decrease the mass ([kappa] > 4), the total current starts showing divergences (Figure 6(d)). The point of divergence is given by (14). The average of a plateau between two divergences is at some multiple of [I.sub.sat] and located at integral values of flux. The width of the plateau decreases with the decrease of mass (Figure 6(e)). As we go to the massless limit (Figure 6(f)), the total current appears as sharp pulses at integral values of flux.
5. Susceptibility of a Many Electron Ring
The total susceptibility is evaluated by taking the flux derivative of the total current. It is well known that superconducting rings are perfect diamagnets and so are the mesoscopic metalic rings. Let us see the nature of the susceptibility for the relativistic fermions.
The change of the magnetic susceptibility with mass is quite interesting for relativistic fermions (Figure 7). For large mass the susceptibility is negative and almost constant (Figure 7(a)). The ring behaves as a diamagnet like a superconducting ring. As we decrease mass, it starts showing periodic oscillation with negative amplitude (Figures 7(b), and 7(c)) with period [[PHI].sub.0]. The maxima are located at integral flux values. The susceptibility becomes zero at critical mass (Figure 7(d)) with a sharp divergence at half integral values of flux which are due to change of step height in flux-current relationship curve (Figure 6(c)). As we further decrease the mass, the periodic oscillation appears again, but this time with positive amplitude (Figures 7(e) and 7(f)). The susceptibility has a minimum value at integral flux and encounters a positive divergence at half integral values of flux. The positive magnetic susceptibility is also reported for carbon nanotube torus  where the electrons behave as massless Dirac fermions. To understand the dependence of susceptibility on particle mass, it is better to focus on the vicinity of an integral value of flux. Here we choose [PHI] = 0 and study the variation of susceptibility both with respect to mass and ring radius.
One can have a better idea about the change of susceptibility with respect to mass from (Figure 8(a)). For large mass, we see that the susceptibility is negative and varies little with mass. This is the nonrelativistic limit where the rings behave as diamagnets. The susceptibility increases with the decrease of mass and becomes zero at critical mass. On further decrease of mass, the susceptibility becomes positive and keeps increasing as we proceed to the zero mass limit many particle fermionic rings thus make a smooth diamagnetic to paramagnetic transition with decrease of mass. One must have noticed that for single particle susceptibility, the real governing parameter is [kappa] (9) which is proportional to the inverse of the product of m and R (11). Hence the same behaviour of total susceptibility can be observed if one keeps m fixed and tune R. We choose a fixed value of the particle mass (m = lme) and plot the total susceptibility against the ring radius (R) (Figure 8(b)) and we find the nature to be similar to that of the total susceptibility, mass curve (Figure 8(a)). The zero susceptibility occurs at R = R(tm) which is half the reduced Compton wavelength of the particle (15). Thus from Figure 8(b), we can easily see that for larger radius, the ring will be diamagnetic whereas smaller rings will be paramagnetic.
6. Possible Experiment
In this paper we have discussed everything keeping mass as a parameter. But for experimental purpose variation of particle mass is not a very useful idea. One can alternatively fix the mass and vary the radius (R) of the ring. The critical radius ([R.sup.m.sub.cri]) 15) at which the single particle current becomes constant ([I.sub.sat]) and consequently susceptibility becomes zero is found to be half of the reduced Compton wavelength of the particle. But designing such small ring is a great challenge and in this way we cannot go to the massless limit either. On the other hand, doped graphene can be a good testing ground for such experiment. On a pure graphene sheet, electrons behave as massless Dirac fermions. In case of a doped graphene, there is band gap [40-42], which corresponds to a massive Dirac fermion. The band gap can be controlled by the doping concentration. Thus instead of mass, one can use doping concentration as the driving parameter. Another way to introduce a mass gap in energy spectrum is to grow the graphene sheet on different substrate . By controlling the mass gap, it may be possible to study the nature of the persistent current. However confining electron in a one dimensional ring in graphene would be a great challenge. Due to Klein tunnelling, potential barriers will not be sufficient for confinement. The edge of a graphene disk can provide a one-dimensional path, but due to edge effect, the physics would be different from that of a simple Dirac fermion.
In this paper, we thoroughly study the nature of persistent current for relativistic fermion. From our analysis, it is clear that the current is a sensitive function of the particle mass as well as the radius of the ring. For large mass, the total current is linear in flux with constant negative susceptibility. But as we move to low mass regime, the behaviour is more and more nonlinear which is clearly shown in Figure 6. We find the existence of a critical mass ([m.sup.R.sub.cri]) below which the energy becomes imaginary which indicates unstable states for certain range of flux. The current shows a divergence within this range. Even more interesting is the nature of the susceptibility. For large mass, it is negative and constant like a nonrelativistic case. As we go to low mass regime, the susceptibility appears to be a periodic function of flux with periodicity Oq (Figure 7). Not only that, its amplitude also increases with the decrease of mass. At m = [m.sup.R.sub.cri] (k = 4) the susceptibility becomes zero (Figure 7(d)) and gradually turns positive with further decrease in mass. The same behaviour can also be observed if we fix the mass and vary the ring radius (Figure 8(b)). We show that a ring with bigger radius (R > [R.sup.m.sub.cri], where [R.sup.m.sub.cri] is half the reduced Compton wavelength of the particle (15)), is diamagnetic while that with smaller one (R < O is paramagnetic.
The author likes to thank Alexander Altland for helpful comments. The work is financially supported by the Council of Scientific and Industrial Research, India.
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S N Bose National Centre for Basic Sciences, Block JD, Sector III, Salt Lake, Kolkata 700098, India
Correspondence should be addressed to Sumit Ghosh; email@example.com
Received 22 April 2013; Revised 9 October 2013; Accepted 2 December 2013
Academic Editor: Sergio E. Ulloa
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|Title Annotation:||Research Article|
|Publication:||Advances in Condensed Matter Physics|
|Date:||Jan 1, 2014|
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