# Intrinsic oscillations of spin current polarization in a paramagnetic resonant tunneling diode

## Abstract

A spin- and time-dependent electron transport has been studied in
a paramagnetic resonant tunneling diode using the self-consistent
Wigner-Poisson method. Based on the calculated current-voltage
characteristics in an external magnetic field
we have demonstrated that under a constant bias both the spin-up
and spin-down current components exhibit the THz
oscillations in two different bias voltage regimes. We have shown
that the oscillations of the spin-up (down) polarized current
result from the coupling between the two resonance states: one
localized in the triangular quantum well created in the emitter
region and the second localized in the main quantum well. We have
also elaborated the one-electron model of the current
oscillations, which confirms the results obtained with the
Wigner-Poisson method. The spin current oscillations can lower the
effectiveness of spin filters based on the paramagnetic resonant
tunneling structures and can be used to design the generators of
the spin polarized current THz oscillations that can operate under
the steady bias and constant magnetic field.^{1}

###### pacs:

72.25.Dc, 85.30.Mn## I Introduction

Dilute magnetic semiconductors (DMSs) such as ZnMnSe and GaMnAs are promising materials due to their potential applications in spintronics.(1); (2); (3); (4); (5); (6); (7) The recent homo- and heteroepitaxy methods(8); (9); (10); (11); (12); (13); (14); (15) allow to deposit the DMS layers with thicknesses of few nanometers, which enables to fabricate spintronic nanodevices with the spin polarization of the current being controlled by the external magnetic and electric fields.

The spin filter based on the DMS was proposed by Euges.(16) The nanostructure studied in Ref. (16) consisted of a paramagnetic semiconductor layer made from ZnMnSe sandwiched between two non-magnetic ZnSe layers. The external magnetic field leads to the giant Zeeman splitting of the conduction band minima in the paramagnetic layer, which causes that this layer acts as a potential well for spin-down electrons and a potential barrier for spin-up electrons. As a result, the total current flowing through the nanostructure is dominated by the spin-down electrons. In such a spin filter,(16) the change of the spin polarization of the current requires the change of the external magnetic field. In the recently fabricated paramagnetic resonant tunneling diodes (RTDs)(17); (18); (19), the electrical control of the spin polarization of the current has been achieved. The spin-polarized current is controlled by the bias voltage in the presence of the external magnetic field in paramagnetic RTDs(17); (20); (21); (18) or even without the external magnetic field in ferromagnetic RTDs.(22); (23); (24); (25); (26); (27) If the quantum well in the RTD is made from the DMS, the spin splitting of the quasi-bound state energy level gives rise to the resonant tunneling conditions for the spin-up and spin-down electrons satisfied for different bias voltages. This leads to the separation of both the spin current components and consequently to the spin polarization of the net current. The operation of the paramagnetic RTD based on ZnSe/ZnBeSe/ZnMnSe heterostructure as a spin filter has been experimentally demonstrated by Slobodskyy et al.(17) and theoretically described by Havu et al.(28) Recently, the spin polarization of the current in the paramagnetic RTD has been reported at zero magnetic field.(18) All these studies of the spin-polarized currents in the magnetic RTDs were devoted to the stationary (steady) currents. The oscillations of the spin-polarized currents in magnetic RTDs have not been studied until now, although the intrinsic oscillations of the current have been detected in the non-magnetic resonant tunneling structures.(29); (30); (31)

The intrinsic current oscillations occurring in the non-magnetic RTDs are intensively studied due to their potential application as THz generators. Recently, the THz oscillations have been experimentally observed in the GaInAs/AlAs RTD integrated with a slot antenna.(29); (30); (31) The attempts undertaken in order to explain the origin of these oscillations led to contradictory conclusions. Ricco and Azbel(32) argued that the oscillations of the current in the non-magnetic RTD result from the fact that the system enters and leaves the resonant current conditions. According to this model,(32) the intrinsic oscillations of the current should occur at the resonance bias that is in contradiction with the experimental(29); (30); (31) and numerical(33) studies, which show that the current oscillations occur only in the negative differential resistance (NDR) regime of the current-voltage characteristics, i.e., above the resonance bias. Woolard et al.(34) suggested that the current oscillations in the non-magnetic RTD result from the charge fluctuations in the potential well created between the emitter and the nearest barrier. This proposition was extended by Zhao et al.,(35); (36); (37) who showed that the intrinsic oscillations are due to the coupling between the quasi-bound state localized in the emitter-related quantum well and the quasi-bound state in the main quantum well. However, this model(35); (36); (37) is based on the adiabatic approximation, according to which the electron states are slowly varying in time. This assumption is not valid in the THz oscillation regime. Moreover, the explanation given by Zhao et al.(35); (36); (37) does not answer the question, why the current oscillations do not decay in time as a result of the dissipative factor corresponding to the imaginary part of the resonance state energy. In our recent paper,(38) we have shown that the intrinsic oscillations of the spin-unpolarized current result from the coupling between the two arbitrary quasi-bound states in the non-magnetic triple-barrier resonant tunneling structure. We have found the intrinsic oscillations in two bias ranges. We have interpreted the oscillations that occur at the bias values below the resonance bias as resulting from the coupling between the quasi-bound states in both the quantum wells, while the oscillations that occur in the NDR regime as resulting from the coupling between the emitter-related quasi-bound state and the quasi-bound state localized in the nearby quantum well.

In the present paper, we study the spin- and time-dependent electronic transport in the paramagnetic double-barrier RTD based on ZnSe/ZnBeSe/ZnMnSe. We show that – under certain well-defined constant bias and external magnetic field – the intrinsic oscillations of both the spin current components appear, which leads to the oscillations of the spin polarization of the total current. Based on the analysis of the spin- and time-dependent potential energy profiles and electron density distributions, we demonstrate that the oscillations of the spin polarized current result from the coupling between the quasi-bound state localized in the triangular quantum well created in the emitter (E) region with the spin-dependent quasi-bound state localized in the main quantum well (QW). The present results show that at certain bias voltages the spin polarization of the current flowing through the paramagnetic RTD is not constant but oscillates with the THz frequency. This effect can be of crucial importance for the possible applications of this nanodevice as a spin filter and THz generator.

The paper is organized as follows: in Sec. II, we describe the theoretical model of the paramagnetic RTD and the time-dependent Wigner-Poisson method. Section III contains the results, Section IV – the discussion, and Section V – conclusions and summary.

## Ii Theoretical model

We consider the spin-dependent electronic transport through the paramagnetic RTD that consists of the paramagnetic quantum-well layer made from ZnMnSe embedded between the two barrier layers made from ZnBeSe (Fig. 1). The active (undoped) region of the nanodevice is separated from the -doped ZnSe ohmic contacts by the two spacer layers made from ZnSe. In the presence of the external magnetic field applied in the growth () direction, the exchange interaction between the conduction band electrons and the Mn ions leads to the giant Zeeman splitting of the conduction band minimum in the paramagnetic quantum-well layer.(1) In the external magnetic field, the conduction-band electrons form the Landau states with the wave functions spread over the plane. Therefore, the one-electron problem can be separated into and coordinates and the electronic transport between the emitter and collector can be described as the one-dimensional motion of the electron in the direction.

In order to simulate the electronic transport through the nanostructure, we apply the time-dependent Wigner-Poisson approach, according to which the conduction band electrons are described by the spin-dependent Wigner distribution function.(39); (40); (41) The quantum kinetic equation takes on the following form(39)

(1) | |||||

where is the spin-dependent Wigner distribution function, is the -component of the wave vector, is the electron conduction-band effective mass, and is the spin index.

The non-local potential for spin channel is given by the formula

(2) | |||||

where is the spin-dependent potential energy, which can be expressed as the sum of the two terms

(3) |

In Eq. (3), the first term denotes the spin-dependent potential energy of the conduction-band bottom, while the second term is the potential energy of an electron in the electric field acting in the nanostructure and has the form

(4) |

where is the potential energy of an electron in the electric field generated by voltage applied between the emitter and collector and is the Hartree energy that takes into account the electron-electron interactions. In Eq. (3), we have neglected the exchange energy (see Subsection IV.C).

The conduction-band potential energy profile has the form

(5) |

where and ( and ) are the positions of the left (right) potential barrier interfaces, is the height of the potential barrier, and is the Zeeman energy of an electron in the paramagnetic quantum-well layer, which is positive (negative) for the spin-up (spin-down) electrons. For a small concentration of Mn ions the Zeeman energy can be expressed by the formula(1)

(6) |

where eV is the sp-d exchange constant, is the concentration of Mn ions, is the Brillouin function for spin that corresponds to the spin of Mn ion, is the effective Landé factor, is the Bohr magneton, and are the phenomenological parameters corresponding to the antiferromagnetic interaction between the Mn ions and have been taken on as and K for .(42)

Potential energy satisfies the Poisson equation

(7) |

where is the elementary charge, is the vacuum electric permittivity, is the relative static electric permittivity, is the concentration of the ionized donors, and is the total density of electrons with being the density of the electrons with spin . The energy of the emitter conduction-band bottom is taken as the reference energy and set equal to .

In order to solve the system of non-linear equations (1) and (7) we apply the self-consistent time-dependent procedure(43) with the boundary conditions and for the Poisson equation, where is the length of the nanodevice. For the quantum kinetic equation (1) we apply the generalized form of the boundary conditions proposed by Frensley(44)

(8) | |||||

Distribution function is derived from the Fermi-Dirac distribution function by summing over the Landau energy levels, which leads to

(9) |

where is the temperature, , is the electrochemical potential of reservoir , is the corresponding Fermi energy, is the voltage applied to contact , and is the cyclotron frequency. In Eq. (9), determines the highest occupied Landau state and is determined by the density of electrons in the reservoirs.

The spin-dependent Wigner distribution function allows us to calculate the spin-dependent electron density

(10) |

and the spin-dependent current density

(11) |

The spin polarization of the current is defined as follows:

(12) |

where and are the spin-up and spin-down current densities, respectively.

In the present work, we focus on the oscillations of the spin-polarized currents. In order to choose the nanostructure parameters, for which the current oscillations are mostly pronounced, we have performed a number of computational runs that allowed us to establish the optimal values of the parameters. The present simulations have been performed for the following values of the nanostructure parameters: the thickness of each contact is equal to 17 nm, the thickness of each spacer layer is 3 nm, the thickness of the potential well layer is 5 nm, the total length of the nanodevice nm, and the Mn concentration %. The barriers are assumed to be symmetric with thickness 3 nm each. We have taken on the height of both the potential barriers eV.(45) The contacts are made from the -type ZnSe with the homogeneous concentration of donors cm. Due to the small thickness of the double-barrier region we assume the effective electron mass of the ZnSe conduction band, i.e., , where is the free electron mass. We take on the relative electric permittivity of ZnSe for the entire nanostructure. The present simulations have been carried out for temperature K on the computational grid with mesh points for coordinate and mesh points for -component of the wave vector. The coordinate increment was , where nm is the lattice constant of ZnSe.

## Iii Results

The calculated current-voltage characteristics for spin-up and spin-down components of the current in the presence of the external magnetic field are displayed on Fig. 2. The resonant current peaks for both the spin current components are separated, which results from the fact that the resonance conditions for the spin-up and spin-down electrons are satisfied at different bias voltages due to the giant Zeeman splitting of the quasi-bound state energy levels in the paramagnetic quantum well. If the magnetic field increases the resonant current peak for the spin-down electrons shifts towards the lower bias, while the resonant peak for the spin-up electrons shifts towards the higher bias [Fig. 2(a,b,c)]. The separation of these peaks is the basic property that can be exploited to fabricate an effective spin filter, in which the spin polarization of the current is controlled by the bias voltage. Figure 3 shows the spin polarization of the current as a function of the bias voltage for different magnetic fields. For all values of the magnetic field the spin polarization of the current varies from for the low bias to for the sufficiently high bias. Moreover, for the higher magnetic field the transition between the almost fully spin polarized currents occurs in a narrower bias interval.

The current-voltage characteristics presented in Fig. 2 have been calculated in the bias range from to V with step V. For each step, the bias voltage has been changed to the next value by if both the spin current components reach the steady state as shown in inset (A) of Fig. 2(a). We have found that at certain bias voltages that belong to the NDR regimes for the spin-up and spin-down electron currents both the spin currents do not stabilize as the steady currents but oscillate with the THz frequency [cf. inset (B) on Fig. 2(a)].

In Fig. 4, we present the formation of the current oscillations for the bias V that corresponds to the NDR regime for the spin-down current component [Fig. 4(a)] and V that corresponds to the NDR regime for the spin-up current component [Fig. 4(b)]. In both the cases, the spin-polarized current oscillates with constant frequencies equal to THz for V and THz for V. For the bias voltages, for which the current oscillations have been found, the spin current polarization is not well defined but also oscillates with the THz frequency. Figure 5 displays the oscillations of the spin current polarization that occur in the NDR regime for the spin-down [Fig. 5(a)] and spin-up [Fig. 5(b)] current component. We note that the spin current polarization exhibits the oscillatory behavior in the bias regimes, in which it reaches the maximal values.

In order to get a physical insight into the mechanism of oscillations of the spin-polarized currents, we have calculated the time- and space-dependence of the electron density in the different regions of the nanostructure (Figs. 6 and 7). Figure 6 shows the time dependence of spin-up and spin-down electron densities in the emitter region and in the main quantum well (QW) calculated for the bias corresponding to the NDR regimes for spin-down and spin-up current components. We see that both the spin-up and spin-down electron densities oscillate with the constant frequencies that are equal to the frequencies of the oscillations of the corresponding spin-polarized current. Figure 6(a) shows that in the NDR regime for the spin-down current component, the amplitude of the spin-down electron density oscillations in the QW region is much larger than the corresponding amplitude of the spin-up electron density oscillations. At time instant , the spin-down electron density reaches the maximal value in the QW region and the minimal value in the emitter region. On the other hand, at time instant , the spin-down electron density is minimal in the QW and maximal in the emitter region [cf. Fig. 6(a)]. The similar behavior has been obtained for the spin-up electron density in the corresponding NDR regimes for the spin-up current component [Fig. 6(b)].

Figure 7 depicts the spatial distribution of the spin-up and spin-down electron densities together with the corresponding self-consistent potential energy profiles determined at time instants and marked on Fig. 6.

Figure 7(a) shows that the density of the spin-down electrons in the QW is fairly large at time instant and much smaller at . These changes of the spin-down electron density in the QW mean that the tunneling conditions at time instants and are different. Therefore, the spin-down current component approaches (at ) and partially leaves (at ) the resonant tunneling conditions. At these time instants, the density of the spin-up electrons in the QW is considerably smaller and oscillates with smaller amplitude [Fig. 7(a)]. In this case, the low-amplitude oscillations of the spin-up electron density are induced by the high-amplitude oscillations of the spin-down electron density [cf. Fig. (6(a)]. Similar results have been obtained for the spin-up electron density in the QW for the bias corresponding to NDR regime of the spin-up current component [Fig. 7(b)]. At time instant the spin-up electron density in the QW is larger than at time instant . At these time instants, the density of the spin-down electrons in the QW is considerably smaller and changes only slightly during the oscillations [Fig. 7(b)]. This indicates that the spin-down polarized current is out of the resonance, which explains the small values of the spin-down current in the considered bias regime.

## Iv Discussion

The results of Sec. III show that – for the paramagnetic RTD in the external magnetic field – we can expect two bias voltage regimes, in which the spin polarization of the current is not well defined but oscillates with the THz frequency. Figure 2 shows that the oscillations of the spin-polarized current are generated in the two following bias ranges: the first corresponding to the NDR regime for the spin-down current component and the second corresponding to the NDR regime for the spin-up current component. The present results obtained for the paramagnetic RTD resemble those for the non-magnetic RTD, (33) according to which the current oscillations occur only in the NDR regime of the current-voltage characteristics. The previous studies (29); (30); (31); (35); (36); (37) of the current oscillations in the non-magnetic RTD allow us to conclude that the occurrence of this phenomenon does not depend on the spins of electrons flowing through the nanostructure. In the next subsections, for simplicity and without loss of generality, first we propose the model of the spin-independent current oscillations in the non-magnetic RTD and next extend this model to the description of the spin-polarized current oscillations in the paramagnetic RTD.

### iv.1 Model of current oscillations

In this subsection, we will analyze the current oscillations using the one-electron approximation. In order to explain the origin of the oscillations, let us consider the physical processes occurring in the NDR regime. In this regime, the system leaves the resonant tunneling conditions, which means that the probability of the reflection of the electron from the emitter barrier becomes fairly large. The interference between incident and reflected electron wave functions together with the bias-induced lowering of the electron potential energy leads to the formation of a shallow triangular quantum well in the emitter region (cf. Fig. 7), in which the quasi-bound (resonance) state is formed. Let us consider the coupling between the resonance state mainly localized in the triangular quantum well in the emitter region and the resonance state localized in the QW. In the framework of the proposed model, we will calculate the probability of transition from state to state under influence of the weak perturbation corresponding to the change of the bias and show that this probability oscillates in time.

The one-electron wave function evolves in time according to the time-dependent Schrödinger equation

(13) |

where potential energy is a functional of the wave function, which results from the wave-function representation of the electron density that in turn determines the potential energy via Poisson equation (7). Potential energy can be expressed as the sum of three terms

(14) |

where is the potential energy of the electron in the steady state for the bias that corresponds to the maximum of the resonant tunneling current. The Hamiltonian with potential energy describes the unperturbed system. The next two terms in Eq. (14) correspond to the perturbation, where is the change of the electron potential energy caused by varying the bias from to () and is the corresponding change of the Hartree potential energy.

The change of Hartree potential energy results from changing the potential energy of the electron in the external electric field by amount and occurs with some time delay with respect to . Moreover, is much smaller than , and therefore, in the first approximation, it can be neglected when considering the electron states at the bias .

In order to avoid the exponential divergence of the resonance wave function in Eq. (13) all the calculations will be performed using the complex-scaling theory of resonance states. (46) The complex-scaled Hamiltonian of the electron has the form

(15) | |||||

where is the scaling parameter(46) and is the Hamiltonian of the unperturbed system for the bias .

In the NDR regime, i.e., for , the resonance states and are almost degenerate, i.e., . Therefore, the one-electron wave function can be expressed as a linear combination of the wave function being localized in the emitter region and localized in the QW

(16) |

Wave functions are calculated using the time-independent Schrödinger equation for the unperturbed Hamiltonian

(17) |

where the energy of the resonance state consists of the real part that determines the position of the resonance on the energy scale and the imaginary part that defines the width of the resonance and determines its lifetime.

After inserting (16) into the time-dependent Schrödinger equation (13) we obtain

(18) |

where

(19) |

Finally, the wave function takes on the form

(20) | |||||

where are the time-independent coefficients,

(21) |

(22) |

and

(23) |

If we take the resonance state as the initial state of the system, i.e., the state for and , the probability of transition from state localized in the emitter quantum well to state localized in the QW is expressed by the formula

(24) |

where

(25) |

The probability of the electron transition from the QW to emitter is given by

(26) |

Based on Eqs. (24) and (26) we state that the coupling between the resonance states localized in the emitter and in the QW (measured by ) causes that the probabilities of the electron transition between the both resonant states oscillate with frequency . As a consequence of this coupling, both the electron density and the current density oscillate in certain well-defined bias intervals in the NDR regime. Eqs. (24) and (26) show that the densities of electrons localized in the emitter and in the QW regions oscillate in anti-phase, which supports the results presented in Fig. 6.

### iv.2 Spin current oscillations in the paramagnetic RTD

Based on the results of Sec. III and Subsection IV. A we argue that the oscillations of the spin-polarized currents in the NDR regimes result from the coupling between the spin-dependent quasi-bound state localized in the emitter region with the corresponding spin-dependent quasi-bound state localized in the main QW.

Now we will analyze the formation of the oscillations of the spin-down polarized current in the NRD regime of the current-voltage characteristics for this current component [cf. Fig. 2(a)]. In this regime, the resonant tunneling conditions for the spin-down electrons are no longer satisfied and the reflection probability of these electrons from the emitter barrier becomes fairly large. Due to the interference and the bias-induced lowering of the potential energy, the spin-down quasi-bound state of the electron is formed in the triangular quantum well in the emitter region close to the left barrier [cf. Fig. 7(a)]. We have estimated the energy of this resonance state to be meV. This energy differs by few meV from energy of the resonance state localized in the QW. Therefore, these states can be treated as almost degenerate and we can apply the results of Subsection IV. A. The coupling between these two quasi-bound states leads to the oscillatory transitions of the spin-down electrons between the emitter and QW regions [cf. Fig. 6(a)] described by the Eqs. (24) and (26). The oscillatory changes of the spin-down electron density in the QW causes that the bottom of the QW oscillates in time, which gives rise to the oscillatory changes of the tunneling conditions. Figure 8(a) shows the transmission coefficient as a function of incident electron energy at time instants and marked on Fig. 6(a).

The positions of the peaks of correspond to the energies of the spin-up and spin-down resonance states localized in the main QW. Figure 8(a) shows that at time instant the resonance tunneling condition is satisfied for the spin-down electrons, which leads to the accumulation of these electrons in the QW [Fig. 7(a)]. After 1 ps the system gets out of the resonance and the density of the spin-down electrons in the QW decreases reaching the minimal value at time instant [cf. Fig. 7(b)]. As a consequence, the spin-down polarized current oscillates [cf. Fig. (6(a)]. For this bias voltage, the oscillations of the spin-up electron density are induced by the electron-electron interactions with the oscillating spin-down electron density.

The same effect, i.e., the coupling between the two spin-up resonance states, one localized in the emitter quantum well and the second localized in the QW, is responsible for the oscillations of the spin-up polarized current that occur in the NRD regime for this current component [cf. Fig. 2(a)]. This coupling leads to the oscillatory exchange of the spin-up electrons between the emitter and the QW, which changes the tunneling conditions in an oscillatory manner.

### iv.3 Effect of exchange interaction

The results presented in Sec. III have been obtained without the exchange interaction [cf. Eq. (3)]. We have also studied the effect of exchange interaction on the oscillations of spin polarized currents. For this purpose we have estimated the exchange energy in the QW using the formula(47) , which leads to meV for the time instant, for which charge density reaches the maximal value during the oscillation cycle. Inserting this formula to Eq. (3) we have calculated the spin-dependent current-voltage characteristics and obtained very similar results to those presented in Fig. 2(a). In particular, we have found two bias regimes, in which THz current oscillations appear. The estimated frequency of these oscillations is smaller than that calculated without the exchange interaction, but still remains in the THz range. We conclude that the exchange interaction can lead to a slight modification of the current-voltage characteristics, but does not affect the predicted occurrence of the high-frequency spin current oscillations.

## V Conclusions and Summary

In the present paper, we have shown that – in the paramagnetic RTD under constant bias and external magnetic field– the stable oscillations of the spin-polarized current can occur in the NRD regimes for the spin-up and spin-down current components. The analysis performed in Sec. IV reveals that these oscillations result from the coupling between the spin-up (spin-down) resonance state localized in the emitter region with the spin-up (spin-down) resonance state localized in the quantum well. This coupling leads to the oscillatory changes of both the electron density and the current in the nanostructure.

In the RTD under the fixed bias and external magnetic field, we deal with the following two types of the spin-polarized currents: (i) stationary (constant in time) current with the well-defined spin polarization, (ii) oscillating current with the oscillating spin polarization. We have demonstrated that at a certain bias in the NDR regime, at which the spin polarization of the net current reaches the maximum, the spin current polarization oscillates with the THz frequency.

Until now the THz oscillations of the current have been observed only in non-magnetic resonant tunneling diodes(29); (30); (31) but they should be also occur in paramagnetic resonant tunneling diodes. We hope that the present results will stimulate the experimental search for this phenomena in the magnetic resonant tunneling structures. We would like to mention that the oscillations of the spin-polarized currents are fully manifested only if the scattering on phonons and impurities is negligibly small, i.e., this is the low-temperature effect. The scattering processes will damp the oscillations and finally lead to the steady current.

The oscillations of the spin-polarized currents, predicted in the present paper, can have important implications for spintronic devices based on the paramagnetic RTD. The separation of both the spin components of the current is a basis for a fabrication of an effective spin filter (selector), in which the spin polarization of the current is controlled by the bias voltage. However, if the paramagnetic RTD is designed to operate as a spin filter, we have to avoid the bias regimes, in which the current oscillations appear, in order to obtain the well-defined spin polarization of the current. On the other hand, the current oscillations obtained under the constant bias can be applied to generate the spin-polarized current oscillating with the THz frequency.

In summary, we have demonstrated that the spin-polarized current flowing through the paramagnetic RTD under the constant bias fixed in the NDR regime and in the constant external magnetic field can exhibit the THz oscillations. The oscillatory behavior of the spin-polarized current leads to important consequences for the operation of spintronic devices. On the one hand, this phenomenon is disadvantageous for the operation of spin filters as a parasitic effect that spoils the operation of spin filters. On the other hand, it can be used to design the generator of the spin-polarized currents oscillating with the THz frequency.

###### Acknowledgements.

This paper has been supported by the Foundation for Polish Science MPD Programme co-financed by the EU European Regional Development Fund and the Polish Ministry of Science and Higher Education and its grants for Scientific Research.### Footnotes

- To be published in Phys.Rev.B.

Copyright (2012) by the American Physical Society.

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