Apr 30, 2012 - ward the center of the wire, the length scale of the expo- nential drop, Î¾ â 30 a .... nels (Noc) as functions of the chemical potential Âµ for a fixed Zeeman .... imate quite well the numerical data (red empty circles). The agreeme
Oct 18, 2008 - presence of impurities, compared to that of the pure system. PACS numbers: 81.05. ... the system including the electronic density of states.11,12.
Feb 16, 2014 - We found that there exist mid-gap energy bands induced by the vortex superlattice and the mid-gap energy bands have nontrivial topological properties including the gapless edge states and non-zero winding number. An topological anisotr
Apr 1, 2011 - however, known that some degree of universality can be recovered by performing sample (or disorder) .... where Ln(z) is the Laguerre polynomial of degree n. This kernel is also known as the form factor in the ...... 76, 499 (1996); A. H
Jun 25, 2013 - ... on the DOS, for electron and phonon systems . ... For phonons the situation is different, because one ..... Communications 4, 1793 (2013).
arXiv:cond-mat/9509137v3 30 Oct 1995 ... (September 8, 1995). Abstract .....  M. F. Crommie, C. P. Lutz and D. M. Eigler, Nature 363, 524 (1993); Science 262,.
Aug 30, 2011 - Analyzing the dispersion relations and the spectrum of the linear chain we show that the excess of low frequency modes, the analog of the boson peak in glassy disordered systems, arises from the strong coupling between rotations and tr
Jul 9, 1999 - have nontrivial quantum corrections due to both nesting and elastic impurity scattering processes, as a result the van Hove singularity is preserved in the center of the band. However, the energy ... host atoms of the lattice. Then, the
Aug 29, 2017 - Abstract. Quadratic bosonic Hamiltonians over a one-particle Hilbert space ... tected states also appears in other physical systems described by wave equations. ... this Krein space structure for the spectral analysis of the BdG ...
We present a numerical study of the quasi-particle density of states (DoS) of two-dimensional d- ... marize some key features of the system: Each node ac-.
Dec 23, 2013 - of states (LDoS) in disordered two-dimensional electron gases (2DEG) in the quantum Hall regime, .... electronic states. These disorder effects can be well cap- tured within a semi classical picture33â37 involving a nat- ural decompo
Nov 9, 2010 - a Majorana edge mode preserving the time reversal symmetry. We calculate topological invariant number and discuss the relevance to a single Majorana edge mode. In the presence of the Majorana edge mode, the SDOS depends strongly on the
Aug 29, 2011 - for F.5 In experiments using strong ferromagnets, the re- sults have been less clear.13,14 At this time, to the best of our knowledge, there is no ...
supercurrent, leading to a modification of the DOS and to a reduction of the gap. .... field created by the supercurrent has a negligible effect: for Is = 70 ÂµA in the ...
them the DOS and the critical temperature of the superconducting transition Tc were analyzed in the âdirty limitâ. This means that the ..... Here MS = (klÂµ)2 + Îº2 s.
Nov 12, 2014 - 1Graduate School Materials Science in Mainz, Staudingerweg 9, 55128 Mainz, Germany. 2Institut fÃ¼r Physik, Johannes Gutenberg-UniversitÃ¤t Mainz, Staudingerweg 7, 55128 Mainz, Germanyâ. 3Physikalisches Institut, Goethe-UniversitÃ¤t F
When a normal metal is in contact with a superconductor, pairing correlations appear on the normal side. The proximity effect ... In this Letter we focus on this last aspect by considering the case in which the metal is an itinerant ferromagnet. ...
Jan 17, 2001 - quantum wires for all ten pure Cartan symmetry classes. The anomalous ...... 18 T. Senthil, M. P. A. Fisher, L. Balents, and C. Nayak,. Phys. Rev.
Nov 7, 2007 - tial approximation (CPA),30,34 the corresponding results are appropriate to address the electronic structures of graphene with an extreme low ...
Apr 30, 2018 - (Dated: May 2, 2018). The Brillouin zone of the clean Weyl semimetal contains points at which the density of states (DoS) vanishes. Previous work suggested that below a certain critical concentration of impurities this feature is prese
Jan 17, 2001 - the DOS whereby the wire is closed by a perfectly reflecting wall on the right. ...... R. Gade and F. Wegner, ibid, 360, 213 (1991). 10 A. Furusaki ...
Nov 25, 2014 - Gil Young Cho,1 Rodrigo Soto-Garrido,1 and Eduardo Fradkin1, 2. 1Department of ... 2Kavli Institute for Theoretical Physics, University of California Santa Barbara, CA 93106-4030, USA ... d-wave SC state in the pseudogap regime [9, 13â
Mar 21, 2016 - with a Chern number C = 4 to a topological phase with C = 1, in the disordered system ..... performed using CLUMEQ/McGill HPC supercomput-.
Density of states of disordered topological superconductor-semiconductor hybrid nanowires Jay D. Sau1 and S. Das Sarma2 1
arXiv:1305.0554v1 [cond-mat.mes-hall] 2 May 2013
Department of Physics, Harvard University, Cambridge, MA 02138 2 Condensed Matter Theory Center and Joint Quantum Institute, Department of Physics, University of Maryland, College Park, Maryland 20742-4111, USA. Using Bogoliubov-de Gennes (BdG) equations we numerically calculate the disorder averaged density of states of disordered semiconductor nanowires driven into a putative topological p-wave superconducting phase by spin-orbit coupling, Zeeman spin splitting and s-wave superconducting proximity effect induced by a nearby superconductor. Comparing with the corresponding theoretical self-consistent Born approximation (SCBA) results treating disorder effects, we comment on the topological phase diagram of the system in the presence of increasing disorder. Although disorder strongly suppresses the zero-bias peak (ZBP) associated with the Majorana zero mode, we find some clear remnant of a ZBP even when the topological gap has essentially vanished in the SCBA theory because of disorder. We explicitly compare effects of disorder on the numerical density of states in the topological and trivial phases. PACS numbers: 03.67.Lx, 03.65.Vf, 71.10.Pm
The theoretical prediction1–6 that the combination of spin-orbit coupling, Zeeman spin splitting, and ordinary s-wave superconductivity could lead to an effective topological superconducting phase under appropriate (and experimentally achievable) conditions has led to an explosion of theoretical and experimental activities6 in semiconductor nanowires (InSb or InAs) in proximity to a superconductor (NbTi or Al) in the presence of an external magnetic field. The experimental finding7 of a ZBP, in precise agreement with the theoretical predictions in the differential tunneling conductance of an InSb nanowire (in contact with a NbTiN superconducting substrate) at a finite external magnetic field (B ∼ 0.1−1 T), followed by independent corroborative observation8–11 of such ZBP both in InSb and InAs nanowires in contact with superconducting Nb and Al by several groups, has created excitement in the condensed matter physics community as well as the broader scientific community as perhaps the first direct evidence supporting the existence of the exotic, the elusive, and the emergent unparied Majorana bound state in solids. Such excitement has invariably been followed by a wave of skepticism as one would expect in a healthy and active scientific discipline with questions ranging all the way from whether such ZBP could arise from other (i.e. non-Majorana) origin to whether all aspects of the observed experimental phenomenology are consistent with the putative theoretical predictions on the topological superconductivity underlying the existence of the Majorana mode. One particular issue, which is also the subject of the current work, attracting a great deal of theoretical attention12–24 is the role of disorder in the Majorana physics of superconductor-semiconductor hybrid structures. Disorder plays a key role in the Majorana physics because the underlying topological super-
conducting phase hosting the Majorana mode (at defect sites) is essentially an effective spinless p-wave superconductor1–5 , which, unlike its s-wave counterpart, is not immune to non-magnetic elastic disorder (i.e. spin-independent momentum scattering) as was already known ten years ago25 . Thus, even the simplest kind of disorder, namely zero-range random non-magnetic point elastic scatterers in the wire, could strongly affect the topological superconductivity in contrast to ordinary s-wave superconductivity which is immune to nonmagnetic disorder, and the associated Majorana bound states by suppressing the (topological) superconducting gap13 and/or creating Andreev bound states in the superconducting gap near zero-energy14 complicating the observation and the interpretation of the ZBP. We do, however, mention that elastic disorder or momentum scattering in the superconductor itself, no matter how strong (as long as it does not destroy the superconductor), does not affect the topological superconducting phase in the semicondutor.21 In addition, it has recently been emphasized that elastic disorder by itself could create a zerobias peak (essentially, an anti-localization peak associated with the disorder-induced quantum interference) in the non-topological phase in the presence of spin-orbit coupling and Zeeman splitting. Since the precise topological quantum critical point (as a function of the applied magnetic field) separating the topological and the trivial superconducting phase is in general not known in the experiments,7–12 one cannot be absolutely sure that the observed ZBP is indeed a Majorana bound state (MBS) signature in the topological phase and not a trivial antilocalization peak in the non-topological phase. In the current work we consider disorder effects on MBS physics by directly calculating the density of states (DOS) of finite disordered nanowires in the presence of proximity-induced superconductivity taking into account spin-orbit coupling and spin splitting arising respectively from Rashba and Zeeman effects in the wire.
2 We use random uncorrelated point scatterers with δfunction potential in the wire to represent the elastic disorder. The theory follows the standard prescription26 of an exact diagonalization of the BdG equations in a minimal tight-binding model including superconducting pairing, Rashba spin-orbit coupling, and Zeeman splitting in the Hamiltonian. The diagonalization of the discretized tight-binding Hamiltonian leads to the exact eigenstates of the system, which then immediately give the density of states (theoretical details are available in Ref. 26 and are not repeated here.) Comparison with theory in the presence of disorder neccessitates the ensemble averaging over many different impurity configurations since each disorder configuration produces its own unique result with random impurity-induced delta-function peaks in the superconducting gap.
λ = 18 μm
λ = 2 μm
λ = 5 μm
λ = 1 μm
λ = 0.5 μm
λ = 0.2 μm
λ = 0.07 μm
λ = 0.03 μm
DOS IN THE DISORDERED TOPOLOGICAL PHASE
In this section, we consider the effect of disorder on the SM/SC system starting from the topological phase in the clean limit. In Fig. 1 (with 8 panels, each representing a different strength of disorder keeping all other parameters fixed), we show our numerical DOS as a function of energy (E) for different relevant parameter sets in the topological phase of the system. We show both the ensemble averaged DOS using many-impurity configurations(but using the same disorder strength, i.e. the same impurity density and potential strength, changing only the random localitions of the impurities along the wire) and the typical DOS for a single impurity configuration in each case. Each panel corresponds to a specific disorder strength (i.e. a fixed impurity density) and shows results for three different lengths of the nanowire. Since our calculations follow either Ref. 26 for the exact numerical treatment of Ref. 13 for the SCBA theory, we refer the reader to those references for the technical details, which are actually pretty standard.19–22 The superconductor (SC)-semiconductor (SM) hybrid nanowire structure is characterized by a large number of independent parameters, both for the actual experimental laboratory systems and for our minimal theoretical model. The minimal set of parameters necessary to describe the system are the proximity-induced SC gap (∆0 ) in the SM, the parent SC pairing potential (∆s ), the Rashba spin-orbit coupling (αR ), the spin splitting (VZ ), the chemical potential (µ), the SM effective mass (m) which defines the SM tight-binding hopping parameter, the nanowire length (L), and disorder (which we take to be the uncorrelated random white noise potential associated with randomly located δ-function in real space spin-independent scattering centers). There are a few additional physically important parameters which are, however, not independent parameters of the theory: the coherence length in the nanowire (ξ), the SM mean-free path (λ) due to disorder, and the number of
FIG. 1. Disorder averaged density of states in the topological phase for the semiconductor nanowire in a magnetic field with Zeeman splitting VZ = 5 K, proximity-induced pairing potential of amplitude ∆0 = 3 K, Rashba spin-orbit coupling strength αR = 0.3 eV − ˚ A. For this choice of parameters the clean quasiparticle-gap ∆ = 1.3 K and coherence length ξ = 0.3 µm. The difference panels (a-h) correspond to different disorder strengths characterized by Es = ~/2τ = 10, 50, 100, 200, 460, 1300, 3300, 7300 mK. The corresponding mean-free paths are λ are in the panels and the self-consistent Born gaps ESCB = 1.2, 1.1, 0.9, 0.8, 0.13, 0, 0, 0K.
occupied subbands (i.e. transverse quantized levels) in the nanowire which we take to be one throughout assuming the system to be in the one-dimensional limit. (The single sub-band approximation, made entirely for the convenience of keeping the number of parameters in the model to be tractable, is a nonessential approximation, and our qualitative results should be completely independent of this approximation.) In addition, there is an independent parameter defining the hopping amplitude across the SC/SM interface which controls the proximity-induced SC pairing gap ∆0 in the SM in terms of the parent gap ∆s in the SC. Finally, the proximity gap (∆) in the SM in the presence of spin-orbit cou-
3 pling and finite Zeeman splitting is reduced from ∆0 in a known manner. All the details for modeling the disorder are given in Ref. 13 where SCBA was used in contrast to our exact numerical diagonalization in the current work following Ref. 26. One specific goal of our current work is to compare the analytic and simple SCBA theory13 with the exact tight-binding numerical analysis to test the limits of validity and the applicability of the SCBA theory which, being analytic, can be used rather easily. We choose parameters approximately consistent with the InSb/Nb systems studied experimentally in7 . These are : ∆0 = 3K, αR = 0.3eV − ˚ A (corresponding to an 2 effective spin-orbit coupling strength m∗ αR = 2.5K). Since out interest is in disorder effects, we focus on a range of magnetic fields with a spin splitting VZ ∼ 5K (we vary it in a few cases only to change the proximity to the topological quantum phase transition point, separating the topological and the trivial SC phase). Given that the condition for the topological SC phase to be realized in the SM is given by2 VZ > ∆2 + µ2 , where ∆ is the actual induced gap in the SM, the system should be in the MBS carrying topological phase for ∆ < 5K (since µ = 0). Given that ∆ < ∆0 = 3K, with the reduction of ∆ below ∆0 arising from the existence of VZ 6= 0, our system is deep in the topological phase for the results shown in Fig.1 since VZ (= 5K) ∆(= 1.3K) and µ = 0. Each panel in Fig. 1 corresponds to a different disorder strength in the system, characterized by the corresponding level broadening Es = ~/2τ (where τ is the scattering time – τ = ∞ in the absence of disorder) or equivalently the mean free path λ = vF τ (where vF is the fermi velocity), both calculated in the SCBA according to Ref. 13 for the given disorder in the wire. In each panel (and for each disorder) we show our DOS numerical results for two distinct wire lengths L = 1.5 µm and L = 3 µm. In each case, we show both the ensemble averaged DOS results using an averaging over many (> 1000) random impurity configurations (keeping Es , λ etc fixed) and the result for a typical single impurity configuration (the distinct crosses or dots denoting delta functions for the DOS at the value of energy ). We emphasize that for an infinitely long wire (L ξ ≈ 0.5 µm for our case) the DOS in the absence of disorder will vanish throughout the gap (±1.3 K in our case) with a δ-function peak at E = 0 associated with the MBS at the wire edges. To characterize the disorder strength for the results in Fig. 1 (with panels (a) to (h) with increasing disorder keeping all other parameters fixed ), we use SCBA for this problem which was developed by us in Ref. 13. The SCBA theory provides us with the SC gap in the topological phase for a given disorder strength, allowing us to compare our direct (and exact) numerical calculation in the presence of disorder with the SCBA theory. We show the calculated SCBA gap in each case in the figure captions for the sake of direct comparison with the exact results in the figures. (The SCBA theory is obviously an ensemble averaged theory for the infinite system and does not depend on L.) It is clear from the result of Fig.
1 that the analytical SCBA theory of Ref. 13 are in excellent qualitative agreement with the exact ensembleaveraged numerical results for the DOS even for Es ≈ ∆, where the topological gap essentially vanishes (panel (e) in Fig. 1) both according to the SCBA (i.e. ESCB = 0) and in our numerical results. While the disorder averaged DOS calculated by exact diagonalization does not stricly vanish inside the gap, the gap calculated with the SCBA can be identified with the peaks in the DOS at the edges of the gap. The closing of the gap within the SCBA coincides with the disappearance of the dips in the DOS around zero-energy. The DOS peak at E = 0 associated with the MBS is continuously suppressed with increasing disorder, but quite amazingly there is a discernible DOS peak at E = 0 even for Es (= 3.3K) ∆(= 1.3K) where ESCB = 0, and at best the topological superconductivity is gapless. The remarkable result, which is quite apparent in our Figs. 1 (e)-(g), is that the MBS peak of the DOS at E = 0 is actually very robust to disorder and survives disorder strength substantially larger than that (typically Es ∼ ∆) destroying the induced superconducting gap ∆. Thus, in Figs. 1(e)-(g), although the SCBA theory and our exact numerical results both show the system to be gapless with Es > ∆, the DOS peak at E = 0 associated with the MBS persists until Es ∆ as in Fig. 1(h) where Es = 7K( ∆ = 1.3 K). It is not only that the MBS feature in the ensemble averaged DOS survives up to very strong disorder (e.g. the mean free path λ = 0.5 µm, 0.2 µm and 0.06 µm respectively in Figs. 1(e)-(g) which are smaller than the wire lengths of L = 1.5 µm and 3 µm used in our numerical work), the typical DOS for single random impurity configuration also shows peaks at E = 0 as can clearly be seen in Figs. 1(e)-(g) [ and as well as in Figs. 1(a)-(d)], but not in Fig. 1(h) where the very large disorder strength (λ = 0.02 µm) suppresses both the ensemble averaged MBS peak as well as the single configuration peak at E = 0. The survival of the zero-energy DOS peak well above the point where the SC gap is completely suppressed by disorder is an important new result of our exact numerical work directly establishing the possible theoretical existence of a gapless topological SC phase.
The origin of the E = 0 peak in the DOS in the strongly disordered case can be related to the Griffiths effect previously considered for the spinless p-wave superconductor25 . The Griffiths effect in the semiconductor nanowire at finite VZ arises from the disorder-induced variation of the chemical potential, which can lead to a transition from a topological phase to a non-topological phase and vice-versa. The variation of the effective chemical potential can lead to domain-walls between topological and non-topological regions each of which would support a local zero-energy MBS. Since each region is of
4 finite extent, the MBSs are a finite distance apart and split into conventional states with a non-zero energy. In fact, by carefully considering the distribution of the distances between the MBSs, it has been shown25 that this splitting typically leads to a singular peak in the DOS at E = 0, which diverges as E → 0 as a power-law in E. The topological phase is of course characterized by true zero-energy edge states, whose energy is exponentially small in the length of the system L. Thus, in the long wire limit, the topological phase and the non-topological phase both have power-law divergent DOS due to the Griffiths effects, but the topological phase has a pair of zero-modes exponentially close to zero energy12 . This distinction between exponential versus power-law in the length seems to appear in the DOS plotted in Fig 1. At small disorder, there is a sharp peak which is very weakly split. At larger disorder (panels (e,f,g,h)) , which is approximately when the gap vanishes i.e. ESCBA → 0, the E ∼ 0 peak in the DOS is broadened. For finite length systems, the sharp transition between the topological and non-topological phase at finite disorder becomes a crossover. While the topological invariant can be computed even for a disordered, but strictly infinite system12,23,24 , we have not done so in the present work because we restrict ourselves to systems of wire lengths comparable to the experimental systems. For such finite wires the distinction between the topological and non-topological phase is not sharp. In fact, the zeromodes arising from the Griffiths effect are themselves MBSs. The MBSs characterizing the topological phase are special only in the sense that they occur near the ends of a finite system and are therefore separated from other low-energy MBSs by a distance of the order of the length of the wire. This can also occur from the Griffiths effect in some realizations of disorder, even in the non-topological parameter regime. Therefore, the Griffiths singularities seen in the disordered Fig. 1 indicate the presence of several low-lying MBSs in the spectrum of the finite wire. For very large disorder the system becomes completely non-topological (and gapless) as in Fig. 1(h). There are three important messages following from our DOS results for the topological phase in the presence of disorder: (1) the zero-energy DOS peak associated with the MBS is strongly suppressed by disorder; (2) SCBA is an excellent quantitative approximation for calculating the SC gap in the topological phase including effects of disorder; and (3) most importantly, the zero-enenrgy MBS peak is very robust against disorder and survives well after the SC gap in the topological phase has been suppressed to zero, and disappears only when the mean > free path λ < ∼ ξ/6 or Es ∼ 6∆ (for the systems are studied) whereas the topological SC gap vanishes for λ < ∼ ξ. Given the quantitative validity of the SCBA, we can calculate the phase diagram of the SC/SM structure in the presence of disorder by using the analytical SCBA theory.13 We show our SCBA-calculated quantum phase diagram of the system in Fig. 2. In Fig. 2, we fix all pa-
FIG. 2. Quasiparticle gap ∆ (in the color bar) versus Zeeman potential VZ and scattering rate Es in the topological phase. The black region represents the gapless phase and is therefore not topologically robust.
rameters except for disorder (Es ) and spin-splitting (VZ ) with the color representing the calculated SC gap ESCBA in the presence of disorder (by definition ESCBA = ∆ for Es = 0). The black region represents gapless superconducivity. We note, based on our numerical results of Fig. 1, that a large part of the black region in the phase diagram allows for well-defined zero-energy DOS MBS peaks although the system is essentially a gapless topological superconductor in this regime. Much of this SCBA gapless regime is dominated by Griffiths physics except for very large disorder when the system eventually becomes nontopological (i.e. even the finite topological segments disappear). Much of this SCBA gapless regime is dominated by Griffiths physics except for very large disorder when the system eventually becomes non-topological. Except for our current results showing the well-defined robust persistence of the MBS peak even in the gapless topological regime (the black region in Fig. 2), one would have concluded that SCBA predicts a rather gloomy picture for the existence of the Majorana mode in the disordered SC/SM hybrid structure since, without our current exact results, the conclusion would have been that there cannot be any MBS in the black region of the phase diagram. Of course the quantitative details of the SCBA phase diagram depend on the SOcoupling strength and the topological phase with a large SC gap is easily achieved by large (small) SO coupling (disorder).
III. DOS IN THE DISORDERED NON-TOPOLOGICAL PHASE
Next we comment on the effect of disorder in the nonp topological SC regime, i.e., for VZ < ∆2 + µ2 for the
FIG. 3. Disorder averaged density of states in the nontopological phase for the semiconductor nanowire in a magnetic field with Zeeman splitting VZ = 0, 1 K (panels (a, b) respectively) at µ = 0 for different disorder strengths characterized by scattering rates Es = ~/τ .
FIG. 4. Disorder averaged density of states in the topological phase for the semiconductor nanowire in a netic field with Zeeman splitting VZ = 4, 5 K (panels respectively) at µ = 5 K for different disorder strengths acterized by scattering rates Es = ~/τ .
nonmag(a, b) char-
SC/SM hybrid structure. In Fig. 3(a) and (b), we show our calculated numerical DOS in the non-topological SC phase (for µ = 0) for VZ = 0 (3a) and 1K (3b) in the presence of disorder. All parameters other than VZ are exactly the same as in Fig. 1. We see that, at least for µ = 0, the behavior of the DOS is similar to a classic s-wave SC (even for VZ = 1 K which simply reduces the gap from ∆0 = 3 K to 2 K) with essentially no discernible effect on the DOS. Even for disorder as large as Es > 7 K > 2∆0 , we do not see any structure developing in the SC DOS gap which remains completely flat. For VZ = 0 (Fig. (3a)) this is a direct consequence of Anderson’s theorem where the robustness of the gap arises from time-reversal symmetry. We see in Fig. (3b) that this behavior persists for small Zeeman fields as long as VZ < ∼ ∆. This behavior can be expected based on previous studies on the bound states of single impurities in spin-orbit coupled nanowires in proximity to superconductors27 . There
it was found that the low-energy sub-gap states appear for short-ranged impurities only in the topological phase. However, this conclusion might not apply to longer-range disorder because in principle, at any non-zero value of Zeeman potential puddles can lead to the formation of a pair of low-energy MBSs. In our numerical work here we restrict ourselves only to zero-range white noise disorder in the semiconductor. The situation, however, changes qualitatively when we consider the limit VZ > ∼ ∆. We show these results in Fig. 4 where VZ = 1 K, µ = 5 K and VZ = µ = 5 K are shown for several values of the disorder parameter Es (≡ ~/2τ ). All other parameters are the same as in Fig. 1 and 2. We note that the situation in Fig. p 4 describes the non-topological phase since VZ = µ < µ2 + ∆2 . In both panels, large disorder has a strong effect on the SC DOS shrinking the SC gap considerably. However, in Fig. 4(b), where VZ ∆, eventually for Es = 0.2 K
6 p VZ = µ2 + ∆2 condition cannot be satisfied except for ∆ = 0 (i.e. VZ → ∞)– but, even the nontopological SC is strongly affected by disorder (for VZ ∆) here since the combination of spin-orbit coupling and Zeeman splitting makes the Anderson theorem moot. Thus the DOS peak in Fig. 4, associated with anti-localization,16–19 arises purely in the trivial phase with a completely suppressed quasiparticle gap which might enable its experimental distinction from the MBS peak in the topological SC phase.
FIG. 5. Quasiparticle gap (∆) versus Zeeman potential VZ for different values (µ = 0, 5K) for the chemical potential µ. The vanishing of the quasiparticle gap marks the topological quantum phase transition from the non-topological phase at small VZ to the topological phase at large VZ .
and 1.3 K (and VZ = µ = 5 K), the DOS seems to ”flip” and the dip at E = 0 becomes a peak at E = 0 with a concomitant vanishing of any SC gap feature in the data. For even larger Es (Es = 7 K in Fig. 4) the peak feature in the DOS is suppressed, but there is a clear E = 0 DOS peak for intermediate (but still large with Es > ∆) disorder (Es = 0.2 K and 1.3 K in Fig. 4) where the SC gap has disappeared, but a peak has developed in the DOS at zero-energy. We believe that the zero-energy DOS peak in Fig. 4(b) for Es = 0.2 K and 1.3 K has the same origin as the physics recently discussed in several publications16–18 . The hallmark of this ”trivial” DOS peak (arising from the competition among spin splitting, spin-orbit coupling, and superconductivity) are that (1) it arises only for large Zeeman splitting in the non-topological phase; (2) it occurs only after the SC quasiparticle gap has been completely suppressed by disorder; (3) it exists only in an intermediate disorder range where the superconducting quasiparticle gap has been suppressed, vanishing for larger disorder and the peak becoming a dip (i.e. the SC gap) for smaller disorder. In order to specify where precisely in the phase diagram we are obtaining our exact numerical results in the presence of disorder we finally show in Fig. 5 our calculated SC gap as a function of VZ (for zero disorder) for the parameters chosen in our calculations. For µ = 0 (i.e. Figs. 1-3), the topological quantum phase transition (TQPT) happens at VZ = ∆0 (= 3 K in our choice), and our Fig. 1 belongs to the topological phase (VZ = 5 K, to the right of the TQPT) whereas our Fig. 2 belongs to the non-topological (VZ = 0, 1 K) to the left of the TQPT. Results for Fig. 4 are obtained for VZ = µ (and VZ < µ) which never can manifest a TQPT since the
Finally we mention that the spin-orbit coupled semiconductor system thus has two distinct topological quantum phase transitions in the presence of the superconducting proximity effect and Zeeman splitting. The first one is driven by the Zeeman field as originallyp predicted by Sau et al2 with the TQPT defined by VZ = µ2 + ∆2 assuming a low disorder situation. The second one is driven by increasing disorder (Es ) in p the finite Zeeman splitting situation (i.e. VZ > µ2 + ∆2 ) where the topological SC phase is destroyed by disorder (for Es > ∼ ∆), leading to a gapless non-topological phase dominated by the Griffiths physics as originally envisioned by Motrunich et al25 . Since the effective SC gap for VZ 6= 0 depends on VZ , and in particular, ∆ ∝ VZ−1 for VZ ∆0 [see Refs. 5 and 13 for details], we expect that there are two distinct magnetic field driven TQPTs in the semiconductor nanowires - - the first one is the TQPT predicted in Ref. 2–5 taking the system from the trivial s-wave SC (induced by proximity effect) to the (effective p-wave) topological Majorana carrying p−wave SC phase at low disorder (i.e. ∆ Es ), and then the second one at much higher Zeeman splitting (so that ∆ < ∼ Es ) where disorder drives the system from a gapless topological SC to a nontopological Griffiths phase. It is unlikely that this second (purely disorder driven) TQPT would be experimentally accessibly since the gapless nature of the SC phase (i.e. black region in Fig. 2 or the situation corresponding to Fig. 1 (e)-(h)) would make the finite temperature of the experimental system behave like a very high temperature (i.e. T ∆), making any experimental study of this disorder-driven TQPT difficult, if not impossible. Thus, the effective gapless nature of the system in Fig. 1(e)-(g) would make it very unlikely that the DOS peak (which is quite obvious in our theoretical results) could be studied experimentally. The best hope for the direct experimental study of the MBS physics is therefore to have a large SC gap (as in Fig. 1(a)-(d) or in the nonblack region of Fig. 2) in the topological phase which necessitates having low effective disorder (Es ∆), a condition guaranteed by having very clean semiconductor wires and or/very strong SO coupling in the material. We add here that our theoretical results presented in this paper cannot be compared (or connected) with the experiments in any way since we only calculate bulk DOS
7 of the system, which cannot be directly probed experimentally.
In summary, we have studied the disorder averaged DOS of a disordered spin-orbit coupled nanowire in proximity to a superconductor in both the topological and non-topological parameter regime. The features in the DOS associated with the superconducting gap in the topological phase appear to be in good quantitative agreement with the SCBA from previous work13 . Consistent with previous results13 , we find that the dips in the DOS associated with the quasiparticle gap disappear for
C. W. Zhang, S. Tewari, R. M. Lutchyn, S. Das Sarma, Phys. Rev. Lett. 101, 160401 (2008); M. Sato, Y. Takahashi, S. Fujimoto, Phys. Rev. Lett. 103, 020401 (2009) . Jay D. Sau, R. M. Lutchyn, S. Tewari, S. Das Sarma, Phys. Rev. Lett. 104, 040502 (2010). R. M. Lutchyn, Jay D. Sau, S. Das Sarma, Phys. Rev. Lett. 105, 077001 (2010) . Y. Oreg, G. Refael, F. V. Oppen, Phys. Rev. Lett. 105, 177002 (2010). J. D. Sau, S. Tewari, R. Lutchyn, T. Stanescu and S. Das Sarma, Phys. Rev. B 82, 214509 (2010). See, e.g. T. Stanescu and S. Tewari, arXiv:1302.5433 (2013) for a review; C. W. J. Beenakker, arXiv:1112.1950 (2011); J. Alicea, Rep. Prog. Phys. 75, 076501 (2012);M. Leijnse and K. Flensberg Semicond. Sci. Technol. 27, 124003 (2012). V. Mourik, K. Zuo, S. M. Frolov, S. R. Plissard, E. P. A. M. Bakkers and L. P. Kouwenhoven, Science 336, 1003 (2012). M. T. Deng, C. L. Yu, G. Y. Huang, M. Larsson, P. Caroff, H. Q. Xu, Nano Lett. 12, 6414 (2012). A. Das, Y. Ronen, Y. Most, Y. Oreg, M. Heiblum, H. Shtrikman, Nat. Phys. 8, 887 (2012). A. D. K. Finck, D. J. Van Harlingen, P. K. Mohseni, K. Jung, X. Li, Phys. Rev. Lett. 110, 126406 (2013). H. O. H. Churchill, V. Fatemi, K. Grove-Rasmussen, M. T. Deng, P. Caroff, H. Q. Xu, C. M. Marcus, arXiv:1303.2407 (2013). P. W. Brouwer, M. Duckheim, A. Romito, and F. von Oppen, Phys. Rev. Lett. 107, 196804 (2011); P. W. Brouwer,
relatively modest (Es > ∼ ∆) amounts of disorder. However, a zero-energy peak associated with MBSs generated by the Griffiths effect survives to much higher levels of disorder. The DOS peak associated with different levels of disorder arising from the Griffiths effect starting from the topological phase and the antilocalization peak starting from the non-topological phase appear to be different enough that one might distinguish them qualitatively. Of course, at this point one does not expect a sharp distinction between the peak arising from the Griffith’s effect and the antilocalization effect because they are zero energy peaks in the DOS in the non-topological phase in the same symmetry class i.e. class D. This work is supported by Microsoft Q, JQI-NSF-PFC, and the Harvard Quantum Optics Center.
M. Duckheim, A. Romito, F. von Oppen, Phys. Rev. B 84, 144526 (2011). J. D. Sau, S. Tewari, S. Das Sarma Phys. Rev. B 85, 064512 (2012). A. M. Lobos, R. M. Lutchyn, S. Das Sarma, Phys. Rev. Lett. 109, 146403 (2012). T. D. Stanescu, R. M. Lutchyn, S. Das Sarma, Phys. Rev. B 84, 144522 (2011). J. Liu, A. C. Potter, K.T. Law, P. A. Lee, Phys. Rev. Lett. 109, 267002 (2012). D. Bagrets and A. Altland Phys. Rev. Lett. 109, 227005 (2012). P. Neven, D. Bagrets, A. Altland arXiv:1302.0747 (2013). D. I. Pikulin, J. P. Dahlhaus, M. Wimmer, H. Schomerus, C. W. J. Beenakker, New J. Phys. 14, 125011 (2012). S. Takei, B. M. Fregoso, H-Y Hui, A. M. Lobos, S. Das Sarma, arXiv:1211.1029 (2012). R. M. Lutchyn, T. D. Stanescu, S. Das Sarma, Phys. Rev. B 85, 140513(R) (2012). E. Prada, P. San-Jose, R. Aguado, Phys. Rev. B 86, 180503(R) (2012) ; C. Bena et al arXiv:1301.7420 I. C. Fulga, F. Hassler, A. R. Akhmerov, C. W. J. Beenakker Phys. Rev. B 83 155429 (2011). I. Adagideli, M. Wimmer, A. Teker, arXiv:1302.2612 (2013). O. Motrunich, K. Damle, D. Huse, Phys. Rev. B 63, 224204 (2001). C-H Lin, J. Sau, S. Das Sarma, Phys. Rev. B 86, 224511 (2012) . J. Sau, E. Demler, arXiv:1204.2537(2012).