Dec 2, 2015 - arXiv:1506.01751v3 [cond-mat.str-el] 2 Dec 2015. Electron-hole compensation ... Los Alamos National Laboratory, Los Alamos, New Mexico 87545, USA. (Dated: December 3, 2015) ... A novel electron-hole compensation effect is discussed in t
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May 8, 2014 - This work was supported by CNPq-Brazil. The first author thanks CNPq-Brazil and the University of Brasilia for support and hospitality that he ...
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EPJ manuscript No. (will be inserted by the editor)
arXiv:1806.09394v1 [cond-mat.mes-hall] 25 Jun 2018
Finite length effect on supercurrents between trivial and topological superconductors Jorge Cayao1,a and Annica M. Black-Schaffer1 Department of Physics and Astronomy, Uppsala University, Box 516, S-751 20 Uppsala, Sweden
Abstract. We numerically analyze the effect of finite length of the superconducting regions on the low-energy spectrum, current-phase curves, and critical currents in junctions between trivial and topological superconductors. Such junctions are assumed to arise in nanowires with strong spin-orbit coupling under external magnetic fields and proximity-induced superconductivity. We show that all these quantities exhibit a strong dependence on the length of the topological sector in the topological phase and serve as indicators of the topological phase and thus the emergence of Majorana bound states at the end of the topological superconductor.
1 Introduction The search for Majorana bound states (MBSs) in condensed matter physics has recently spurred a huge interest, further enhanced by its potential applications in topological quantum computation [1,2,3]. In one dimension these exotic states emerge as zero-energy end states in topological superconducting nanowires, which can be achieved by combining common properties such as strong spin-orbit coupling (SOC), magnetic field, and proximity- induced conventional superconductivity [4,5,6]. A quantized differential conductance of high 2e2 /h at zero bias  in normalsuperconductor (NS) junctions is one of the most anticipated experimental signatures of MBSs and has motivated an enormous experimental effort since 2012 [8,9,10,11,12,13], where initial difficulties [14,15,16,17,13,11,12,18,19,20] were solved and high quality interfaces have recently been reported [21,22,23,24,25,26,27,28,29,30]. Despite all the efforts, there is however still controversy in the distinction between Andreev bound states and MBSs as in both cases similar conductance signatures might arise due to non-homogeneous chemical potentials [31,32,33]. It is therefore important to go beyond zero-bias anomalies in NS junctions and study other geometries and signatures [34,29]. For recent reviews see Refs. [35,36] One promising route includes superconductor-normal-superconductor (SNS) junctions based on nanowires which are predicted to exhibit a fractional 4π-periodic Josephson effect in the presence of MBSs [1,37,38], as a result of the protected fermionic parity as a function of the superconducting phase difference φ across the junction. Although the 4π-periodic Josephson effect is difficult achieve as it disapa
pears in thermal equilibrium, SNS junctions have motivated both interesting theoretical studies [39,40,41,42,43,44,45,46,31,47,48,49,50,51,52] and promising experimental activity [53,54,55,56,57]. Another possibility recently considered for further evidence of MBSs is multiple Andreev reflection transport in voltage-biased SNS junctions [58,59,60]. But even without additional voltages and at thermal equilibrium there exists proposals for signatures MBSs in SNS junctions. In particular, supercurrents in finite length SNS junctions, despite their overall 2π-periodicity, have very recently been reported to contain useful information about both the nontrivial topology and MBSs [49,51]. In this work we perform a numerical study of the low-energy spectrum, supercurrents, and critical currents in a trivial superconductor-topological superconductor junction based in nanowires with strong SOC. Our work serves as a complementary study to previous reports where the two finite length S regions in the SNS junction where both in the topological regime [49,51]. We find that, unlike in fully topologically trivial junctions, in the topological phase the low-energy spectrum and current-phase curves are strongly dependent on the length of the topological S, which we can directly attribute to the emergence of MBSs and their hybridization. We also obtain that magnetic field dependence of the critical current is almost independent of the lengths of the superconducting regions in the trivial phase. However, in the topological phase the critical current develops oscillations with the magnetic field. These oscillations are connected to the emergence of MBSs but are reduced with increasing the length of the topological S region as the hybridization overlap of the MBSs is then strongly suppressed. We further see no clear features of the topological transition mainly due to the absence of Zeeman field in the left (trivial) region. The remaining of this work is organized as follows. In Sec. 2 we describe the model for SNS junctions based on nanowires with SOC. In Sec. 3 we discuss the phase dependent low-energy spectrum and in Sec. 4 we calculate and analyze the supercurrents as well as critical currents. In Sec. 5 we present our conclusions.
2 Model We consider a single channel nanowire with strong SOC and magnetic field modeled by [61,62,63,64,65,66,67] H0 =
p2x αR −µ− σy px + Bσx , 2m ¯h
where px = −i¯ h∂x is the momentum operator and µ the chemical potential, which determines the electron filling of the nanowire. Furthermore, αR represents the strength of Rashba SOC while B = gµB B/2 is the Zeeman energy as a result of the applied magnetic field B in the x-direction along the wire, with g being the wire g-factor and µB the Bohr magneton. We use parameters for InSb nanowires, which include the electron’s effective mass m = 0.015me , with me the electron’s mass, and the SOC strength αR = 50 meVnm which is approximately 2.5 larger than the initial reported values  and supported by recent experiments in InSb nanowires [68,69].
For computational purposes, the model given by Eq. (1) is discretized on a tightP P binding lattice such that H0 = i c†i hci + hiji c†i vcj + h.c. , where hiji denotes that v couples nearest-neighbor i, j sites. Here h = (2t−µ)σ0 +Bσx and v = −tσ0 +itSO σy are matrices in spin space, with t = h ¯ 2 /(2m∗ a2 ) being the hopping parameter and tSOC = αR /(2a) the SOC strength. Using open boundary condition the nanowire is
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Fig. 1. (a) The left and right regions of a nanowire with SOC are in contact with s-wave superconductors which induce superconducting correlations into the nanowire characterized by pairing potentials ∆L,R , while the central region remains in its normal state. (b) A magnetic field applied solely to the right sector SR drives it into the topological superconducting phase with Majorana bound states γ1,2 at the ends with localization length ξM .
automatically of finite length. We then assume that the left and right sections of the nanowire are in close proximity to s-wave superconductors. This induces finite superconducting pairing correlations into the nanowire characterized by the mean-field order parameter ∆L,R = ∆e±iφ/2 , where φ is the superconducting phase difference across the junction, while the middle region remains in the normal state. This leads to a SNS junction, where the left S, normal N, and right S regions are of finite length LL , LN and LR , respectively, as schematically shown in Fig. 1(a). We here consider very short junctions, such that LN = 20 nm, and keep same chemical potential µ in all three regions for simplicity. The effective junction is thus set by the finite phase difference between left and right S regions. The numerical treatment of the superconducting correlations are carried out within the standard Nambu representation, see Refs.[49,51]. Furthermore, we assume that the magnetic field B is applied solely to the right S region of the nanowire. The left S and N regions are not subjected to any magnetic field. This allows us to drive the right S region into the topological phase p with MBSs γ1,2 at both its ends for B > Bc as depicted in Fig. 1(b), where Bc = µ2 + ∆2 is the critical field [4,5,6]. For B < Bc the whole system is thus topologically trivial and no MBSs are expected. The MBSs in the right S region are localized to its two end points and decay exponentially into the middle of the S region in an oscillatory fashion with a decay length ξM , developing an spatial overlap due to the finite length LR when LR ≤ 2ξM [70,71,72,18]. It is worth pointing out that we have verified (not shown) that the wavefunction associated to γ1 has a small non-oscillatory tail that decays into N and also slightly leaks into the left S region. Using this model we perform numerical diagonalization to investigate the lowenergy spectrum and supercurrents across many different SNS junctions, in particular varying size of the two S regions, as well as superconducting phase and magnetic field strength.
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1 0 -1 0
1 0 1 0 0.5 Phase difference φ/2π
Fig. 2. Phase dependent low-energy spectrum in the trivial phase B = 0.5Bc (top row) and topological phase at B = 1.5Bc (bottom row). Different panels correspond to different values of the length of the left (LL ) and right (LR ) S regions. Notably, an increase in LR changes the low-energy levels in the topological phase (e), but does not affect the trivial phase (b). Lengths are given in units of 100 nm. Parameters: ∆ = 0.9meV, αR = 50meVnm, µL,R = 0.5meV.
3 Energy spectrum In this section we investigate the evolution of the low-lying energy levels εp in a short SNS junction under a magnetic field applied to the right S region and for different superconducting phases φ. Due to the finite length of the whole SNS structure, the energy spectrum is discrete and Andreev reflections at the junction interface together with a finite superconducting phase difference lead to the formation of Andreev bound states within the energy gap ∆. In very short junctions the spin-orbit coupling does not split the energy levels [73,74,73,58,75,76,51] but a Zeeman field generally does. Most importantly, the lowenergy spectrum acquires a phase dependence that allows the identification of MBSs in the topological phase [49,51]. In Fig. 2 we show the phase dependent low-energy spectrum for different values of the length of the left (LL ) and right (LR ) S regions in the trivial B < Bc (top row) and topological B > Bc (bottom row) phases. In the case of equal and short S region lengths (a, d) the low-energy spectrum is very sparse and exhibits an appreciable phase dependence with a marked difference between the trivial (top row) and topological phase (bottom row). In the trivial phase B < Bc , the low-energy levels behave as conventional Andreev states which tend towards zero energy at φ = π , as seen in Fig. 2(a). However, unlike predicted by the standard theory , the minimum energy at φ = π is here non zero mainly because our junction is away from the Andreev approximation where the chemical potential µ is assumed to be the domi-
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LL=20, LR=3 (c)
-1 0 1
0 1 3 5 0 1 Zeeman field B/Bc
Fig. 3. Magnetic field dependent low-energy spectrum at φ = π for equal S region lengths (a), and larger (b) and shorter (c) right region lengths. Topological phase transition B = Bc is indicated by vertical dashed red lines. Notably, the low-energy spectrum is solely affected by changes in the length of the right S sector. Lengths are given in units of 100 nm. Parameters: ∆ = 0.9meV, αR = 50meVnm, µL,R = 0.5meV.
nating energy scale . The situation is distinctly different in the topological phase in Fig. 2(d), where two levels emerge around zero energy with an energy splitting for all phase differences φ, which becomes largest at φ = π. These are the two MBSs formed at either of the topological SR region. It is the finite overlap of the two MBSs across the SR region that causes the energy splitting away from zero. Indeed, as the length of the topological SR region is increased, the splitting of MBSs is exponentially reduced such it even completely vanishes for very long regions as seen in Fig. 2(e), where the MBSs acquire their zero-energy character irrespective of the phase difference. The increase of LR also introduces more energy levels to the quasicontinuum (dense set of levels above the minigap in (b,c,e,f)), but it notably does not modify the low-energy behavior. Further evidence that the energy splitting in (d) is due to MBSs is acquired by instead increasing the length of the left region (LL ), as done in Fig. 2(c,f). In this case the low-energy spectrum is not altered with respect to the case with equal lengths (a,d). Additional and complementary information is given by the magnetic field dependence of the low-energy spectrum, which we present in Fig. 3 for φ = π and different values of LSL(R) . We directly notice how the the magnetic field dependent low-energy spectrum captures the gap closing and the emergence of MBSs for B > Bc , as well as the MBS hybridization through the oscillatory energy levels around zero energy for B > Bc . The gap closing is here not sharp primarily due to the finite length of the system and but also due to relatively large values of the SOC. Although the SOC does not determine the critical Bc , it does affects the sharpness of the gap closing in finite length systems. We also clearly see that the MBSs energy splitting is sig-
Fig. 4. Phase dependent supercurrents in the trivial B = 0.5Bc (a) and topological phase at B = 1.5Bc (b), as well as and magnetic field dependent critical currents (c). Different curves correspond to different values of LSR,L . Notably, an increase in LR affects the supercurrent and critical currents in the topological phase (b,c), but does not affect the trivial phase (a,c). Lengths are given in units of 100 nm. Parameters: ∆ = 0.9meV, αR = 50meVnm, µL,R = 0.5meV.
nificantly reduced by increasing the length of the topological SR region. However, a similar increase in the length of the trivial left region does not introduce any change in the low-energy spectrum, but only give rise to a dense set of levels around ∆, as seen in Fig. 3(c).
4 Supercurrents and critical currents After the above discussion on the low-energy spectrum we now investigate the supercurrents in the SNS junctions, which can be directly calculated from the discrete Andreev spectrum εp as [77,49] I(φ) = −
ε dε eX p p tanh , h p>0 ¯ 2κB T dφ
where κB is the Boltzmann constant, T the temperature, and the summation is performed over all positive eigenvalues εp of the Hamiltonian described our SNS junction.
In Fig. (4)(a,b) we plot the phase dependence of th supercurrents I(φ) in the trivial B = 0.5Bc (a) and topological B = 1.5Bc (b) phases at T = 0. A general feature
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is that in both the trivial and topological phases the supercurrents are 2π-periodic I(φ) = I(φ + 2π) [49,50,51,52], developing its maximum value close to φ = π/2. This is in contrast to the case considering purely semi-infinite topological junctions which report 4π-periodicity of I(φ) when the system is not allowed to relax to thermal equilibrium for each phase [1,37,38]. In the trivial phase supercurrents acquire a sinelike behavior and do not exhibit any change upon variations of the lengths of either right or left S region, as can be seen in Fig. 4(a). Changing the magnetic field from B = 0.5Bc , but still within the trivial phase, do not alter the magnitude of I(φ) but only introduce a small zig-zag feature around φ = π, similar to Ref. . In the topological phase the overall magnitude of the supercurrents I(φ) are reduced due to the higher magnetic fields, as seen in Fig. (4)(b). More importantly though, I(φ) undergoes an enhancement due to the reduction of the MBSs energy splitting when LR increases. We have verified that for very large magnetic fields B >> Bc , the overall supercurrent is reduced and eventually completely suppressed due to the different pairing symmetries in the trivial (s-wave) and topological (p-wave) superconducting regions . Still, there is a significant region for B > Bc where the enhancement observed in Fig. (4)(b) is still useful to identify the topological phase and its MBSs. Further signatures of MBSs can be acquired from the critical currents Ic , which is simply the maximum supercurrent that flows across the junction, which can be calculated by maximizing the supercurrent I(φ) with respect to the superconducting phase difference φ, Ic = maxφ [I(φ)] ,
where I(φ) is numerically found using Eq. (2). In what follows we solely discuss the zero temperature situation T = 0. In Fig. (4)(c) we present the magnetic field dependence of the critical currents for different values of the lengths of the left LL and right LR S regions. At B = 0 the critical current is finite and maximum, while it decreases as the magnetic field increases. In the trivial phase, forB < Bc , the critical currents are exceptionally independent of variations of LSL,R , as seen in Fig. (4)(c). A very different behavior is observed in the topological phase. First, at B = Bc , Ic is still finite, however, the kink-like feature reported in some previous studies [49,51,52] is absent mainly due to the zero Zeeman field B in the left region. We have verified that the SOC, finite length of the S regions, and induced gap also affect the visibility of such kink at Bc but it is more detrimental the absence of B in the left region. Beyond the topological transition, for B > Bc , the critical current is further reduced and finally vanishes for extremely large magnetic fields, as is seen in Fig. (4)(c). This is due to the incompatibility between the trivial region s-wave and fully p-wave state in the topological region at extremely large magnetic fields. However, much before that, the critical current captures the splitting of MBSs through noticeable oscillations as function of the magnetic field. The oscillations are reduced when the length of the topological sector (right S) increases, an effect purely related to the energy splitting observed in the Zeeman dependent low-energy spectrum in Fig. 2. We can therefore attribute this behavior to the emergence and subsequent hybridization of the MBSs, similar to previous reports when the left and right sectors become topological with four MBSs [49,51]. Taken together, this introduces a strong dependence of the critical current on the length of the topological sector in the topological phase B > Bc , unlike in the trivial phase B < Bc where critical currents are length independent. The length dependence of one of the two S regions can thus be used to determine the topological phase transition.
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5 Conclusions In this work we investigated the finite length effect of the superconducting sectors on the low-energy spectrum, supercurrents, and critical currents in junctions between trivial and topological superconductors based on nanowires with strong Rashba SOC. We demonstrated that the low-energy spectrum and current-phase relationship in the topological phase are strongly dependent on variations of the length of the topological S region, but show now dependence on length for the trivial S region. This effect we were able to trace back to the emergence of MBSs. We also showed that the critical current reveal important information in the distinction between trivial and topological phases and thus offer a straightforward experimental signature for nontrivial topology. In particular, the critical current is essentially completely independent of the length of the superconducting regions in the trivial phase. However, in the topological phase there is both a length dependence and the critical current starts to exhibit notable oscillations, which are reduced as the length of the topological sector increases. The oscillations we were able to attribute to the MBSs at either end point of the topological S and their mutual hybridization. Thus both the current-phase relationship and critical current exhibit features that uniquely identifies the topological phase transition in SNS nanowire junctions. Notably, and in contrast to the elusive 4π fractional Josephson effect, both of these effects are accessible through very standard measurements and thus offers straightforward yet powerful signatures of nontrivial topology and MBSs.
Acknowledgments This work was supported by the Swedish Research Council (Vetenskapsr˚ adet, Grant No. 621-2014-3721), the G¨ oran Gustafsson Foundation, the Swedish Foundation for Strategic Research (SSF), and the Knut and Alice Wallenberg Foundation through the Wallenberg Academy Fellows program.
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