# Electrical control of a confined electron spin in a silicene quantum dot

## Abstract

We study spin control for an electron confined in a flake of silicene. We find that the lowest-energy conduction-band levels are split by the diagonal intrinsic spin-orbit coupling into Kramers doublets with a definite projection of the spin on the orbital magnetic moment. We study the spin control by AC electric fields using the non-diagonal Rashba component of the spin-orbit interactions with the time-dependent atomistic tight-binding approach. The Rashba interactions in AC electric fields produce Rabi spin-flips times of the order of a nanosecond. These times can be reduced to tens of picoseconds provided that the vertical electric field is tuned to an avoided crossing open by the Rashba spin-orbit interaction. We demonstrate that the speedup of the spin transitions is possible due to the intervalley coupling induced by the armchair edge of the flake. The study is confronted with the results for circular quantum dots decoupled from the edge with well defined angular momentum and valley index.

## I Introduction

Silicene chow () is potentially an attractive alternative of graphene Neto09 () for spintronic Zutic04 () applications. The material is characterized by strong intrinsic spin-orbit coupling Liu11 (); Liu (); Ezawa () that should allow for observation of quantum spin Hall effect Liu11 (). Moreover, anomalous Hall effect Ezawa () and its valley-polarized variant Pan14 () as well as giant magnetoresistance Xu12 (); Rachel14 () were predicted for silicene systems. Possible applications to spin-filtering Tsai13 (); szak15 (); miso15 (); nunez16 (); wu15 () were proposed and topological phase transitions in the edge states driven by the perpendicular electric field are expected Ezawa12a (); Tabert13 (); romera (). An operating room-temperature field effect transistor has recently been demonstrated Tao15 () for silicene transfered on AlO dielectric, which relatively weakly perturbs the band structure of silicene near the Dirac points al2o3 (). Deposition on a non-metallic surface Tao15 (); al2o3 (); nonmetal (); nonmetal1 (); nonmetal2 (); nonmetal3 () is necessary, since the metal substrate Vogt12 (); Aufray10 (); Feng12 (); me1 (); me2 (); me3 () masks the electronic properties of silicene.

Spin-orbit coupling is relevant for manipulation and control of single carrier spins confined in quantum dots for applications in quantum information processing Zutic04 (); Komputer (); dl (); kl () since it allows for addressing individual quantum dots by electric fields. In particular, control of the confined spin by AC electric fields is possible with the Rashba spin-orbit coupling that translates the electron motion in space into an effective magnetic field meier () that drives the spin rotations edsr1 (); edsr2 (); edsr3 (). This procedure, known as the electric-dipole spin resonance (EDSR) edsr1 (); edsr2 (); edsr3 (), was implemented in III-V semiconductors edsr4 (); edsr5 (); edsr6 (); edsr7 (); extreme (); stroer () and in carbon nanotubes edsrcnt1 (); edsrcnt2 (); edsrcnt3 () for studies of the spin-related properties of confined electron systems. In the present paper we study the spin-orbit coupling in a silicene flake as a resource for EDSR and we simulate the confined spin flips driven by oscillating electric fields.

The carrier eigenstates in graphene flakes have been extensively studied in the literature gru (); zarenia (); flake1 (); flake2 (); flake3 (); flake4 (); flake5 (); mori (). Besides the significant spin-orbit coupling Liu (); Ezawa () silicene due to the buckling of the crystal lattice buck0 (); Cinquanta12 (); chow () allows for control of the electronic structure with perpendicular electric fields. The perpendicular electric field opens the energy gap ni (); Drummond12 () and shifts the energies of the edge-localized states abdelsalam (); kiku (). The electric fields of the order of 1V/Å are necessary for the silicene bandgap tuning Drummond12 () in particular for applications to room temperature field effect transistors ni () or to spin-filtering Tsai13 ().

For the purpose of the present study we employ a hexagonal flake with armchair boundaries. The armchair termination does not support edge states zarenia () and the energy spectrum contains a well resolved energy gap due to the quantum confinement. The energy gap allows us to focus on a single excess electron confined within the flake and adopt a frozen-valence-band approximation when AC electric fields are applied for EDSR. We find that the spin-orbit coupling component which governs the spectrum is the intrinsic contribution of Kane-Mele km () form which is spin-diagonal and splits the fourfold degenerate ground-state into Kramers doublets with definite projections of the spin on the orbital magnetic moment. In presence of strong perpendicular electric fields the typical spin-flip transitions times are of the order of a nanosecond, and the transitions occur according to the two-level Rabi resonance mechanism. We show that the spin transition times are nonlinear and nonmonotonic functions of the vertical electric field and can be significantly reduced within avoided crossings opened by the Rashba interaction. These avoided crossing occurs in the low-energy spectra in presence of intervalley coupling that is introduced by the armchair edge of the flake revrev (). The conclusion is drawn from modeling of circular quantum dots with a well defined valley index and angular momentum with both - the atomistic tight-binding and the Dirac approximation to the Hamiltonian. Formation of spin-valley doublets by the intrinsic spin-orbit interaction for lifted valley scattering is also discussed.

## Ii Theory

The band structure for silicene deposited on AlO Tao15 () is close to the one of the free-standing silicene al2o3 () near the charge neutrality point. For that reason we use the atomistic tight-binding Hamiltonian for free-standing silicene Liu () in the basis spanned by the spin-orbitals,

(1) | |||||

where the indices run over the ions while and over the spin degree of freedom. In Eq. (1) stands for summation over the nearest neighbor ions and for the next nearest neighbors. The first term of the Hamiltonian describes the nearest neighbor hopping with eV Liu (); Ezawa (). The second term with is the intrinsic spin-orbit interaction km (); km2 () with () for the counterclockwise (clockwise) next-nearest neighbor hopping. The adopted value Liu (); Ezawa () of the intrinsic spin-orbit parameter is meV. The third term in Eq. (1) with introduces the Rashba Liu () interaction due the built-in electric field which results from the vertical shift of the A and B sublattices in silicene, with and the position of the -th ion. The intrinsic Rashba interaction acts for the next nearest neighbors with for the sublattice A and for the sublattice B. For the intrinsic Rashba parameter we take meV Liu (); Ezawa (). The Hamiltonian component with is the extrinsic Rashba term which results from the external electric field perpendicular to the silicene plane or the mirror symmetry broken by e.g. the substrate. The parameter varies linearly with the external field with eV for meV/Å Ezawa (). The last term of Hamiltonian (1) introduces the electrostatic potential due to the perpendicular electric field with with plus for ion in the sublattice and minus for the sublattice, and Å is the vertical shift of the and sublattice planes.

We show below that in order to activate effective spin transitions the perpendicular electric field of the order of 1 V/Å is required. A field this high can be obtained for silicene sandwiched within dielectric between metal gates ni (). The external Rashba interaction introduces also the effect of the substrate. In particular, the energy gap found experimentally in Ref. Tao15 () of 210 meV corresponds to an effective vertical electric field of the order of 1.2 V/Å according to a linear extrapolation of the data of Ref. ni, .

For the Hamiltonian of a general form

(2) |

with the specific hopping parameters defined by Eq. (1), the energy operator which accounts for the external magnetic field oriented perpendicular to the silicene plane follows

(3) | |||||

where the first term introduces the Peierls phase, with the vector potential and the second term is the spin Zeeman interaction with the Bohr magneton and the electron spin factor .

We study the spin flips of the electron confined within the flake by application of an external in-plane AC electric field with the time-dependent Hamiltonian

(4) |

where and are the amplitude and the frequency of the AC electric field, respectively. The maximal considered AC amplitude is V/cmeV/Å.

Once the eigenstates of the stationary Hamiltonian are determined , we use them as the basis for description of the time evolution of the wave function

(5) |

which when plugged into the Schrödinger equation , produces the linear system of differential equations eosika (),

(6) |

that we solve with the implicit trapezoid rule.

For the purpose of the present study we consider a hexagonal silicene flake given in Fig. 1(a) with side length of 18.64 nm. In the rest of the paper we consider a single excess electron in the conduction band and focus on the low-energy part of the spectrum, namely on the energy levels plotted in red within the range indicated in Fig. 2 by the green rectangle. In Figure 2 the spin-orbit coupling was neglected. Moreover, Figure 2 is the only plot where we neglect the Zeeman interaction. We note the following: (i) Without the Zeeman interaction all levels are degenerate with respect to the spin. (ii) All the energy levels marked in red tend to 0th Landau level at high . For the armchair termination of the flake [Fig. 1(b)] no localization of the states near the edge is observed zarenia () hence the missing zero energy level in Fig. 2. (iii) A well defined band gap between the conduction and valence band states near . The maximal potential energy variation due to the field is about 1.2 meV within the flake which is much smaller than the energy gap within the green rectangle in Fig. 2. This allows us to treat the valence band as filled and frozen. For the basis given by Eq. (5) we take up to 30 the lowest-energy states of the conduction band.

(a) | |
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(b) | |

(c) |

## Iii Results and Discussion

(a) | (b) | ||

(c) | (d) | ||

(e) | (f) |

### iii.1 Spectra in the absence of the vertical electric field

The low-energy part of the conduction band spectrum for is given in Fig. 3. Without the spin-orbit interaction [Fig. 3(a)] the structure of the lowest conduction-band energy levels with the ground-state quadruplet and the excited doublet is identical to the one obtained for the hexagonal armchair flakes of graphene – see Fig. 5(a) of Ref. zarenia (); uwaga ().

When the spin-orbit coupling interactions are included [Fig. 3(b)] the ground-state quadruplet [Fig. 3(b)] is split to doublets separated by the energy of meV [cf. Fig. 3(a) and Fig. 3(b)]. The Rashba spin-orbit terms are not resolved in the energy spectrum scale of Fig. 3(b) and the difference between Fig. 3(a) and Fig. 3(b) is entirely due to the intrinsic spin-orbit interaction. The first excited energy level is degenerate only with respect to the spin.

The armchair edge mixes the valleys in the Hamiltonian eigenstates zarenia () and the angular momentum for a hexagonal flake is not a good quantum number (see Section III.5). Therefore, we refer to the separate states by the orientation of the magnetic dipole moments: the orbital moment generated by the electrical currents within the flake and by the spin. In labeling the states we take the values obtained at in the absence of the spin-orbit interactions. Accordingly, the energy levels in Fig. 3 and below are labeled by , a and , for the orbital magnetic moments ”parallel”, ”antiparallel” to the external field or ”none”, respectively.

Figure 4 shows the current distribution in the lowest six energy states. The electron current waka () that flows from spin-orbital to the spin-orbital in the tight-binding wave function is calculated as . Figure 4 shows the currents in the majority spin component of the wave function. The other is generally negligible. Outside avoided crossings opened by the Rashba interaction (see below) the spin is nearly polarized in the direction.

For the excited doublet a current circulation at is observed only when the spin-orbit interaction is present. The currents in the n states induced by the spin-orbit coupling are weak compared to the ones that flow in a and states and require a scaling factor of 4 for presentation in Fig. 4(e,f).

The magnetic dipole moment generated by the silicene flake is associated with the energy variation szafran (), where , is the orbital moment and the spin moment. The magnetic orbital moment results from the current circulation within the flake . In the absence of the vertical electric field the orbital magnetic moment dominates over the spin moment. On the energy scale the latter induces only a relatively small energy level splitting via the spin Zeeman interaction – see the blue and red energy levels in Fig. 3(a).

Based on the above results we find that the splitting of the ground-state quadruplet to doublets separated by in Fig. 3(b) shifts down (up) on the energy scale for states with the orbital magnetic dipole moment parallel (antiparallel) to the spin magnetic moment [see Fig. 3(c)]. The energy of the n states with no orbital magnetic moments [Fig. 3(a)] is only weakly changed when the spin-orbit interactions are included [cf. Fig. 3(a) and (b)]. The spin-orbit interaction introduces a built-in magnetic field which for energy levels shifts the extrema off [Fig. 3(b)] and the current circulation in these states – although weak – no longer vanishes at – see Fig. 4(e,f).

[V/Å] | (a,p)() | n () | [meV] |
---|---|---|---|

0 | 0.5 | 0.5 | 57.7 |

0.125 | 0.843 | 0.800 | 80.5 |

0.25 | 0.941 | 0.916 | 126.8 |

0.5 | 0.982 | 0.974 | 234.4 |

1 | 0.995 | 0.993 | 460.2 |

1.5 | 0.997 | 0.996 | 688.5 |

### iii.2 Transition matrix elements

The rate of the resonant spin flips that can be achieved by the AC electric fields is determined by the transition matrix elements , where and are the wave functions of the initial and final states. Table I lists the absolute values of the matrix elements for the ground state set as the initial one . The initial- and the final-state wave functions can be expressed by contributions of separate sublattices and the spin components . The operator is spin- and sublattice-diagonal, hence . The columns in Table I from the 2nd to the 5th contain the absolute values of the contributions to the matrix elements from the A and B sublattices and the spin components of the integrands. Let us first focus on the upper part of Table I that corresponds to . We can see that all the transitions within the ground-state quadruple – with spin flip or not – are forbidden. Only the transitions from p to n states can be induced by the AC electric field, and the rate of the transition with the spin inversion pn is by five orders of magnitude slower than the spin-conserving transition pn.

Let us look at the contributions over the spins and sublattices for . For the final state a the values of all four separate contributions are negligibly small, of the order of nm. For p the contributions are larger – of the order of nm. Note that the non-zero values of the separate contributions between the states of opposite spins are entirely due to the Rashba interactions which are non-diagonal in . However, for p the contributions from one sublattice are exactly cancelled by the contribution of the other sublattice (upper part of Table I). For the spin-conserving transition to a the separate contributions are large but again cancel over the sublattices.

The vertical electric field lifts the cancellation of the contributions from separate sublattices. The vertical field distinguishes the sublattices and for the field shifts most of the wave function to the sublattice (see Table II). The lower part of Table I indicates the changes to the matrix elements introduced by nonzero . The spin-flipping transition within the ground-state quadruple pp has now only three orders of magnitude lower matrix element than the spin-conserving one. The pa spin-flipping transition has still a negligibly small rate since already the contributions of the sublattices are small.

### iii.3 Energy spectra in the vertical electric field

The current flow, at the atomic scale, occurs along the bonds between the sublattices gru (). Therefore, localization of the wave function on the single sublattice [Table II] hampers the current circulation within the flake. The vertical electric field quenches the currents, the orbital magnetic dipole moment is reduced, and so is the scale of the variation of energy levels with – compare Fig. 3(a) for with Fig. 5(a) for V/Å and Fig. 6(a) for V/Å. In presence of the vertical electric field, avoided crossings of states with opposite spin orientations can be resolved. Figure 5 contains signature of energy levels repulsion between p and n levels [Fig. 5(c)] as well as between a and n [Fig. 5(d)] levels. The avoided crossings involve states of opposite spins but the same current orientation at [cf. Fig 4]. Near the avoided crossings [Fig. 5(b)] the transition matrix element from the ground-state to the states of opposite spin is radically increased. The dependence of the matrix elements on is therefore nonlinear and nonmonotonic.

For V/Å [see Fig. 6(a)] only a single avoided crossing is observed in the spectrum – when the spin-up energy level changes in order with spin-down a energy level. The other crossing no longer occurs, since the p energy level at lies higher than the n levels. In contrast to the results with [Fig. 3] in Fig. 6(a) the main source of the energy variation is the spin Zeeman interaction, and the orbital magnetic moments are very small due to the current quenching noticed above. In this sense, the vertical electric field controls the magnetic properties of the flake as the source of the magnetic dipole moment.

The dependence of the spectrum on the vertical field is summarized for T in Fig. 7. For the vertical electric potential the energy reference level is set in the center between the positions of and sublattices. The energy gap as a function of is given in the last column of Table II. The energy of the lowest-conduction band states is equal to half the energy gap. The gap grows with since the conduction (valence) band states get localized at the sublattice whose electrostatic potential is increased (decreased) by the field. The growth of the n states energy is weaker since their localization on the A sublattice with growing is delayed [Table II]. As a result, the n states enter in between the a and p states for V/Å. Note that the spin-orbit energy level splitting between p and p states only weakly depends on the external electric field.

(a) |

(b) (d) |

(a) | |
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(b) |

(a) | |
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(b) | |

(c) |

(a) | (b) |

(a) | (b) | ||

(c) | (d) |

On the scale of Fig. 7 the contribution of the Rashba terms cannot be resolved. The energy levels near the avoided crossing in Fig. 7(c) are determined mostly by the extrinsic Rashba interaction (). For the intrinsic Rashba interaction excluded () the spectrum of Fig. 7(c) does not change at the scale of the figure. Both Rashba interactions open avoided crossings between the same pairs of states. For the width of the avoided crossing defined as the spacing between the anticrossing energy levels in the middle of the crossing at the scale of , the widths of the avoided crossing in Fig. 7(c) are 45 eV for pn and 31 eV for an. When the external Rashba term is switched off (), the corresponding widths narrow down to 5eV and 3eV, respectively.

In Figure 7(b) with the dotted lines we plotted the matrix elements as obtained for . The locally maximal values of the matrix elements remain the same, only the width of the maxima is reduced. Therefore, a larger precision would be required in order to tune into the avoided crossing with the vertical electric field . For the external Rashba interaction excluded () the matrix elements return to small values at large above the avoided crossings.

For the value of kept unchanged but set to zero the results cannot be distinguished from the ones plotted with the solid lines in Figure 7(b).

### iii.4 The spin resonance

For simulation of the electric dipole spin resonance the external magnetic field of 1T was set to lift the degeneracies. In the initial condition the electron was set in the p ground-state. For the AC electric field of the amplitude and frequency is applied [Eq. (4)]. For each value of we monitored in time the maximal occupation of the excited states of the stationary Hamiltonian by projection of the wave function on the eigenstates basis.

We studied the EDSR for V/Å [Fig. 8] i.e. in the neighborhood of the np avoided crossing (see Fig. 7), and in the center of this avoided crossing for V/Å [Fig. 9]. For V/Å the spin of the eigenstates is polarized parallel or antiparallel to the axis. Within the avoided crossing V/Å [Fig. 9] the spins are no longer polarized.

The results for V/Å in Fig. 8 show wide maxima corresponding to spin-conserving transitions to a and n states. For V/cm, the maximal occupation probabilities of the excited states reach 1 for AC pulse duration of several dozens of ps [Fig. 8(a)] provided that the AC frequency matches the resonance. The spin-flip transitions are resolved later in the simulation and the width of the resonant peaks is smaller. The transition to p state for V/Å is distinctly faster than the one to n. For V/Å the avoided crossing involving p is closer [cf. Fig. 7(b)]. In the conditions of Fig. 8(a) the spin flips occur according to the two-level Rabi resonance.

Figure 8(b) shows the results for the amplitude of the AC field increased to V/cm. The transitions rates to the considered excited states are increased. However, the spin-conserving transitions to a and n become wide and overlap on the scale with each other and with the spin flipping transitions. In Fig. 8(b) the two narrow orange and brown peaks near meV are the two-photon transitions to a and n states at half the resonant single-photon frequency.

In the center of the avoided crossing [Fig. 9] the transitions involving the spin inversion appear now nearly as fast as the spin-conserving transition to a state which is higher in the energy. A wide peak is observed at the energy of the avoided crossing [cf. Fig. 9(a,c) and Fig. 9(b,d)] and a sharp one at the higher energy for the transition to n state off the avoided crossing.

The two-photon spin-flipping transitions are observed for the larger AC amplitude [Fig. 9(d)]. Since the time evolution within the avoided crossing involves more than just two states – the transition does not have the typical Rabi dynamics. None of the states within the avoided crossings has a well defined spin orientation. In consequence, the spin flip probability, which acquires large values already after ps does not reach 100% even for the longest times studied. Nevertheless, the present results indicate that one can tune the external static fields to conditions in which the Rashba interactions – notoriously weak in silicene Ezawa () – can be harnessed for fast spin transitions. These transitions should produce a strong signal in the EDSR spectra by effective lifting of the Pauli blockade of the current edsr1 (); edsr2 (); edsr3 (); edsr4 (); edsr5 (); edsr6 (); edsr7 (); extreme (); stroer (); edsrcnt1 (); edsrcnt2 (); edsrcnt3 (). The fast spin flips run by electric pulses should be useful for experimental studies of the spin structure and interactions. A workpoint for the two-level Rabi dynamics outside the avoided crossings can also be selected.

The results of this work are obtained for the side length of the hexagonal flake of nm. We checked how the size of the hexagonal flake influences the conditions and the dynamics of the EDSR. For that purpose we considered a smaller flake with side length nm and a larger one with nm. The spin-orbit coupling splitting at is meV, 3.05 meV and 3.03 meV for , and respectively. The magnetic field for which an avoided crossing of n – a energy levels strongly depends on the size of the flake, and equals 23.7 T, 8.73 T and 3.25 T, for , and respectively. The width of the avoided crossing – involving spin mixing between the states – is smaller for smaller flakes. We attribute this fact to the larger Zeeman interaction for higher . The corresponding widths are 23eV, 28.3eV and 46 eV, in the same order as above. The spin-flip time for the smallest flake with in the center of the n – a avoided crossing for V/cm is 23 ps, of the order found in Fig. 9(b,d).

### iii.5 Circular confinement and removal of the edge effects

The spin flips demonstrated above were accelerated within the range of avoided crossings [cf. Fig. 5(b)] involving the n states which at appear close above the ground-state. In the absence of the spin-orbit interaction and without the intervalley scattering all the energy levels at should be fourfold degenerate: with respect to the valley and the spin. At the ground-state in the hexagonal armchair flake in Fig. 3(a) is indeed fourfold degenerate – with respect to the current orientation and to the spin, but the n states are only twofold degenerate – with respect to the spin only. The twofold degenerate levels at can only result from the intervalley scattering which in the studied flake is induced by the armchair edge. In order to estimate the effects of the intervalley scattering it is instructive to decouple the localized states from the edge.

Moreover, the confined states and the spin-orbit coupling mechanism could be more precisely described in circular confinement using the low-energy continuum approximation gru (); nori (). In this case the angular momentum can be used to characterize the states provided that the intervalley scattering is removed. The reason for the latter is the following. In presence of the intervalley coupling the wave function in the sublattices can be described by

(7) |

and

(8) |

where are the envelope functions corresponding to the valley, and to the valley. The armchair edge does not support localized states, hence at the edge, which implies the boundary conditions on the envelope functions of the form zarenia ()

(9) |

and

(10) |

Since the intervalley distance | is large, the exponent in Eq. (9) oscillates rapidly at the atomic scale and lifts the isotropy of the problem even for a circular edge of the flake.

In this section we introduce a circular confinement and decouple the confined states from the edge. For that purpose we introduce an additional gap modulation nori () within the flake. Namely, we consider a modified Hamiltonian

(11) |

where is defined by Eq. (2). In Eq. (11), for and for . The extra term with widens the energy gap for nori () which results in the carrier confinement for energies close to the Dirac point.

The resulting confinement is illustrated in Fig. 10 for nm. The energy levels that are plotted as functions of turn red when the state gets localized within . In Fig. 10 all the spin interactions are present and T is applied in order to split the degeneracies. We can see that the pair of n energy levels joins two other energy levels at eV and the resulting quadruple moves parallel for larger . The appearance of the quadruple is a signature of lifting the intervalley scattering by separation of the states from the edge. The quadruple is formed by two doublets which at are separated by a large energy spacing of about 70 meV. Only due to the strong intervalley coupling the n energy levels appear low in the energy spectrum close to the ground-state at . The chance for accelerated spin flips at relatively low – where the avoided crossings appear – results from the intervalley coupling.

a) |

b) |

The absolute value of the ground-state wave function on the lattice is displayed for in Fig. 11(a) and for eV in Fig. 11(b). Figure 11(a) contains a checkerboard pattern near the corners of the hexagon and the results of Fig. 11(b) are smooth. The checkerboard results from the rapid wave function oscillations (see Eq. (8)) that follows the intervalley scattering induced by the edge. Even for smooth and , the exponent of Eq. (8) generates rapid variation of the absolute value of . The variation is removed once the coupling of the localized state to the edge is lifted (Fig. 11(b)).

The quantum numbers for the localized states can be conveniently explained in the context of the magnetic field dependence of the energy spectra. For identification of the tight-binding states they are compared to the ones obtained with the continuum approximation Ezawa12a (), for which we keep track of the intrinsic spin-orbit interaction and neglect the Rashba terms. For the vector wave function the continuum Hamiltonian reads Ezawa12a ()

(12) |

with , for valley and for valley, , and is the Fermi velocity, with the nearest neighbor distance Å. , and are the Pauli matrices in the space spanned by the sublattices.

With the symmetric gauge the Hamiltonian eigenstates can be characterized by eigenvalues of the orbital momentum operator , where and is the unit matrix. The eigenfunction is then where is an integer. Summarizing, the continuum Hamiltonian (12) eigenstates have a definite component of the spin, the valley index, and the angular momentum. We label the Hamiltonian eigenstates with quantum number .

Figure 12(a,c) shows the energy spectrum as obtained with the tight-binding approach used above with [Fig. 12(a)] or without [Fig. 12(c)] the spin-orbit coupling for eV. The results of a continuum approach are displayed in Fig. 12(b) without and in Fig. 12(b) with the spin-orbit interaction. The dashed (solid) lines indicate the () valley levels. The results for both approaches are nearly identical and Fig. 12 contains all the information on the corresponding energy levels with respect to both angular momentum, the valley, and the spin. In these conditions one can indicate the mechanism of the spin-orbit coupling more precisely: the spin-orbit interactions splits the fourfold degenerate states of Fig. 12(a,b) to pairs of doublets in the following manner: at in the lower doublet we find and states, and in the higher doublet and states. This form of the spin-orbit coupling splitting is observed in carbon nanotubes kuem ().

In Fig. 12 the energy levels cross the energy levels near 12 T. These crossings are counterparts of the avoided crossings between a,p and n energy levels for the hexagonal flake that increased the spin flip transition matrix element [cf. Fig. 5]. Now, in the tight-binding calculations [Fig. 12(c)] that accounts for the Rashba interaction – we do not resolve any repulsion of the energy levels, or in any case the width of the avoided crossing is smaller than 0.1 eV. The Rashba spin-orbit interaction – that is accounted for in Fig. 12(c) does not open couple energy levels associated to opposite valleys. As far as the transition matrix elements from the ground-state to five lowest-energy excited states in Fig. 12(c) are concerned – the only large one is from to and equals 3.35 nm at . The matrix elements for the spin-flipping transitions as calculated with the atomistic tight binding do not exceed nm.

Based on the result of Fig. 10 and Fig. 12(d) we can see that the n states for the hexagonal flake were mixtures of and states with . We therefore conclude, that the avoided crossing opened by the Rashba interaction in the spectra of hexagonal flake that allowed for the fast spin flips induced by AC electric fields require intervalley scattering.

a) | b) |

c) | d) |

## Iv Summary and Conclusion

We have studied the possibility of the electrical control of the spin for a single excess electron confined within a silicene flake using the Rashba interaction. We found that the transitions within the lowest-energy quadruplet driven by an AC electric field – also the spin-conserving ones – require application of a strong vertical electric field of the order of 1V/Å. For the matrix elements for transitions with or without the spin flip vanish due to cancellation of contributions of separate sublattices. The field lifts the equivalence of the sublattices, the cancellation is no longer complete and the transitions involving both the spin and the orbital degrees of freedom within the quadruplet.

The rate of the spin transitions is a nonmonotonic function of and becomes drastically increased within avoided crossing of the states of the quadruple with the states of the Kramers doublet. The spin flips occur then at the scale of several picoseconds in the external resonant AC field of a low amplitude of the order of hundreds volts per centimeter. However, due to the avoided crossing and the spin-conserving transitions within the same energy range, the induced spin flip is not a selective two-level Rabi transition, but the dynamics involves several eigenstates of the stationary Hamiltonian. Generally, outside the avoided crossings open by the Rashba interaction, the spin transitions occur at a slower rate but with the Rabi two-levels dynamics for the resonant frequency. We found that the properties of the flake as the source of the magnetic dipole moment can be controlled by the vertical electric field which quenches the currents circulating within the flake by localization of the wave function on a single sublattice.

The results were compared to the ones obtained for a circular quantum dot tailored within the flake by the spatial energy gap modulation. The confined states are separated from the edge and the intervalley coupling is removed. Upon removal of the intervalley scattering the avoided crossings that accelerated the spin flips are replaced by crossing of energy levels of opposite valleys and the speedup is no longer observed. Formation of the spin-valley doublets in the absence of the intervalley scattering was demonstrated.

## Acknowledgments

This work was supported by the National Science Centre (NCN) according to decision DEC-2016/23/B/ST3/00821 and by the Faculty of Physics and Applied Computer Science AGH UST statutory activities No. 11.11.220.01/2 within subsidy of the Ministry of Science and Higher Education, The calculations were performed on PL-Grid Infrastructure.

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