Scholarly article on topic ' Enhanced superconductivity due to forward scattering in FeSe thin films on SrTiO 3 substrates '

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Academic research paper on topic " Enhanced superconductivity due to forward scattering in FeSe thin films on SrTiO 3 substrates "

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Enhanced superconductivity due to forward scattering in FeSe thin films on SrTiO3 substrates

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New Journal of Physics

The open access journal at the forefront of physics

Dautsdie PhyilbUiicha GwalUdiaft DPG

IOP Institute of Physics

Published in partnership with: Deutsche Physikalische Gesellschaft and the Institute of Physics

FASTTRACK COMMUNICATION

OPENACCESS

Enhanced superconductivity due to forward scattering in FeSethin films on SrTiO3 substrates

5 November 2015

REVISED

4 January 2016

ACCEPTED FOR PUBLICATION

26 January 2016

PUBLISHED

10 February 2016

Original content from this work may be used under the terms of the Creative Commons Attribution 3.0 licence.

Any further distribution of this work must maintain attribution to the author(s) and the title of the work, journal citation andDOI.

Louk Rademaker1, Yan Wang2, Tom Berlijn3'4 and Steve Johnston2'5

1 Kavli Institute for Theoretical Physics, University of California Santa Barbara, CA 93106, USA

2 Department of Physics and Astronomy, University of Tennessee, Knoxville, TN 37996, USA

3 Center for Nanophase Materials Sciences, Oak Ridge National Laboratory, OakRidge, TN 37831, USA

4 Computer Science and Mathematics Division, Oak Ridge National Laboratory, Oak Ridge, TN 37831, USA

5 Author to whom any correspondence should be addressed.

E-mail: sjohn145@utk.edu

Keywords: superconductivity, electron-phonon interactions, Eliashberg theory, FeSe thin films Supplementary material for this article is available online Communicated by NJP Board member Peter Hirschfeld

Abstract

We study the consequences of an electron-phonon (e-ph) interaction that is strongly peaked in the forward scattering (q = 0) direction in a two-dimensional superconductor using Migdal-Eliashberg theory. We find that strong forward scattering results in an enhanced Tc that is linearly proportional to the strength of the dimensionless e-ph coupling constant 1m in the weak coupling limit. This interaction also produces distinct replica bands in the single-particle spectral function, similar to those observed in recent angle-resolved photoemission experiments on FeSe monolayers on SrTiO3 and BaTiO3 substrates. By comparing our model to photoemission experiments, we infer an e-ph coupling strength that can provide a significant portion of the observed high Tc in these systems.

A flurry of scientific activities has been generated by the discovery of an enhanced superconductivity in FeSe monolayers grown on SrTiO3 (STO) substrates [1-20]. On its own, bulk FeSe has a modest superconducting transition temperature Tc ~ 9 K [21]; however, when a monolayer is grown on an STO substrate, Tc is increased dramatically [ 1]. Most reported Tc values cluster within 55-75 K, close to the boiling point of liquid nitrogen (77 K). (A surprisingly high Tc ~ 107 K has also been reported in in situ transport measurements [9].) This discovery has opened a pathway to high- Tc superconductivity through interface engineering, which has already produced high- Tc's in systems such as FeSe on BaTiO3 (BTO) [8] and FeTe i -*Sex on STO [22].

Determining the origin of the Tc enhancement in these interface systems is critical. At the moment, proposals include charge transfer between the substrate and FeSe [2-4,20], electric field [6] and strain effects due to the substrate [5,8], and lattice related effects such as enhanced electron-phonon (e-ph) coupling in the FeSe layer [1,13,16] or across the interface [7,19]. Strong evidence for the latter has been provided by a recent angle-resolved photoemission spectroscopy (ARPES) study [7], which observed replica bands in the single-particle spectral function of the FeSe monolayer. These replicas are interpreted as being produced by coupling between the FeSe 3d electrons and an optical oxygen phonon branch in the STO substrate. Moreover, the replica bands are complete copies of the corresponding main bands, which implies that the responsible e-ph interaction is strongly peaked in the forward scattering direction (small momentum transfers). Such momentum dependence is notable because it can enhance superconductivity in most pairing channels [23-31]. As such, this cross-interface coupling provides at the same time a suitable mechanism for the Tc enhancement in the FeSe/STO and FeSe/BTO systems [7,8].

We explore this possibility here by examining the consequences of strong forward scattering in the e-ph interaction for superconductivity and the spectral properties of a two-dimensional system. By solving the momentum dependent Eliashberg equations, we show that a pronounced forward scattering results in a Tc that

© 2016 IOP Publishing Ltd and Deutsche Physikalische Gesellschaft

scales linearly with the dimensionless e-ph coupling constant \m (see below) in the weak coupling limit. This is in stark contrast to the usual exponential dependence predicted by BCS theory. Furthermore, this coupling produces distinct replica structures in the spectral function similar to those observed experimentally. By comparing our model to experiments [7], we infer a significant e-ph contribution to the total Tc observed in the FeSe/STO system with a modest value of Am.

1. Formalism

To model the FeSe monolayer we consider a single-band model for the FeSe electron pockets, which includes coupling to an oxygen phonon branch in the STO substrate. The Hamiltonian is given by

H = EXk s ck>+ £Wq fet bq + £ g (k, q) 4+qs ck>a (b!q + bq),

k,s q k,q,s

where ck s (Ck s) and bt (bq) are electron and phonon creation (annihilation) operators, respectively, Xk is the band dispersion, Wq is the phonon dispersion, and g (k, q) is the momentum-dependent e-ph coupling constant.

We calculate the single-particle self-energy due to the e-ph interaction using Migdal-Eliashberg theory. Using the Nambu notation with fermionic Matsubara frequencies wn = (2n + 1) p/b, where b = 1/T is the inverse temperature, the self-energy is SS(k, iwn) = iwn [1 — Z (k, iwn)] t0 + c (k, iwn) t3 + f (k, iwn) t1, where t are the Pauli matrices, Z (k, iwn) and c (k, iwn) renormalize the single-particle mass and band dispersion, respectively, and f (k, iwn) is the anomalous self-energy, which is zero in the normal state. The self-energy is then computed by self-consistently evaluating the one-loop diagram and is given by

S(k, iw„) = —1 £|g(k, q)l2D(0)(q, iw„ — iwm)t)G(k + q, iwm)t),

NP q,m

where D(0)(q, iwn) = — 22Wq 2 is the bare phonon propagator, and G 1 (k, iwn) = iwnt0 — £kt3 — SS(k, iwn) is

the dressed electron propagator.

Migdal's theorem states that the vertex corrections to considerations given above are on the order of 1m (W/ Ef) for a momentum-independent interaction. One might therefore wonder whether the use of Migdal-Eliashberg theory is justified in FeSe/STO, since the ratio W/EF is of order unity. This is bolstered by the fact that Migdal's theorem also breaks down in the limit that the small q scattering processes dominate. In this limit, however, one can show that the vertex corrections are still proportional to the dimensionless coupling 1m [32]. As such, any corrections to the self-energy due to the diagrams neglected in Migdal-Eliashberg theory are of order im, and can be treated perturbatively if the coupling is sufficiently small. As we will show, the value 1m needed to reproduce the ARPES data is small (\m ~ 0.15-0.25), indicating that we are indeedin the perturbative regime. (This is further justified by observing that the contributions to the self-energy from the second order and higher order rainbow diagrams, which are of the same order as the crossing diagrams, are small.) In this context, the work of Pietronero and coworkers is relevant [33,34] as they have studied the contributions of the vertex corrections in the perturbative regime and found that their inclusion serves to increase the superconducting Tc when the e-ph coupling is dominated by small q processes. Based on these considerations, we proceed using Migdal-Eliashberg theory assuming that corrections beyond this approach can be treated at a perturbative level and will likely increase Tc further.

In what follows we parameterize the electronic dispersion as Xk = — 2t [cos (kxa) + cos (kya)] — m with t = 75 meV and m = —235 meV. This choice in parameters produces at r an electron-like Fermi pocket with kF = 0.97/a and a Fermi velocity vF = 0.12eV -a/H alongthe ky = 0line, where a is the in-plane lattice constant. This closely resembles the electron pocket at M point measured by ARPES experiment. Since first principles calculations indicate that the relevant oxygen phonon branch in STO is relatively dispersionless near the T-point [14,35], we approximate the phonon with a flat Einstein mode Wq = W = 100 meV (H = 1),whichis consistent with the observed energy separation of the replica bands [7]. Furthermore, as we are interested in the case of forward scattering, we neglect any potential fermion momentum dependence in the e-ph interaction and set g (q) = g0 exp (— |q|/q0), as microscopically derived before [7,19]. Here, q0 sets the range of the coupling in momentum space. For different values of q0 we adjust g0 to obtain the desired value of the dimensionless e-ph coupling constant 1m, which is computed from the Fermi surface averaged mass enhancement in the normal state \m = (— 9 Re w) |w=0). (We are using 1m to distinguish this definition from the standard one involving a double fermi surface average of the coupling constant |g (k, q) |2. See the supplementary material6 for further details.) Throughout we assume an s-wave symmetry for the gap function, consistent with the observations of a

6 For further details, please see the online supplementary material available at stacks.iop.org/njp/18/022001/mmedia.

fully gapped state on the Fermi level [1,7,10,18]. Finally, we neglect the Coulomb pseudopotential m* in what follows. One should therefore regard our Tc values as upper bounds for the e-ph contribution to the FeSe/STO system. (Some considerations for m* are provided in the supplementary materials6. We find that its inclusion reduces Tc by ~ 20% for typical values of m*.)

2. Analytical results

Before proceeding to full numerical solutions, we can gain some insight by first considering the case of perfect forward scattering, where the e-ph matrix element is a delta function \g (q)|2 = g02 ¿qN with g02 = 1mQ2 (see supplementary material6). In the weak coupling limit, we further set Z (k, iwn) = 1, c (k, iwn) = 0,and therefore f (k, iwn) = A (k, iwn). With these approximations, the gap function on the Fermi surface is given by

. \mQ2 A (iwm) 2Q

A (iWn) = -^—2--7-Tb m Wm + A2(iWm) Q2 + (Wn ~ Wm)

Todetermine Tc we take the ansatz A (iwn) = A0/ [1 + (wj Q)2] and follow the usual steps [37]:thegap equation is linearlized by setting A2 = 0 for T ~ Tc and we set wn=JQ = 0. This results in the condition for Tc

1 1— QQ ^—^ 2

= ~TT ^ w m (i + w2j q2)(Q2 + w m ■

The Matsubara sum can be performed exactly, yielding our final expression

1 = 1mbe 2Q + Q cosh(Qbc) - (3/be)sinh(Qbc) = 2 1 + cosh (Qbe) -

For the case of FeSe, Te ^ Q, and the hyperbolic functions dominate. To the leading order, the critical temperature is quasi-linear in the coupling strength in the weak coupling limit, Te = -—Q. (A similar result

2 + 31m

was obtained in [23] in the context of the cuprates using square-well models.) For 1m = 0-16 and Q = 100 meV one obtains Tc = 75 K, which is a remarkably high temperature for such a modest value of 1m.

The increased Tc should be compared to the standard BCS value obtained for a momentum-independent coupling. In this case, the linearized gap equation simplifies to [36,37]

1 — pTc \m ^ -—- — \„

\wm\<WD\Wm\

H2!t) - -(Î)

where we have expanded at large Qd/T and y (z) is the digamma function (see supplementary material6). This form produces the usual exponential behavior for the critical temperature, Te = 1.13Q exp (-1/ 1m), which predictsaTc = 2.5Kfor 1m = 0.16and QD = 100meV.

Comparing these two results, one sees that the origin of the enhanced Tc lies in the momentum decoupling [24] that occurs in the Eliashberg equations when the interaction is strongly peaked at q = 0. In the BCS case, the integration over the Fermi surface is equally weighted at all momenta, leading to a Y,n term in the BCS gap equation and subsequently a leading logarithmic behavior. In the forward scattering case, there is no integration over momentum so the w-^ term remains, resulting in a leading behavior that scales like 1/ Te (see supplementary material6). Thus, strong forward scattering serves as an ideal mechanism for producing high-Tc superconductivity [30]. Furthermore, a strong forward scattering peak in the coupling constant means that this interaction will contribute in most pairing channels [7,23-31]. It can therefore act in conjunction with other active unconventional channels, providing another means to increase Tc further.

3. Numerical results

In real materials the e-ph interaction is expected to have a finite range q0 in momentum space [7]. Therefore we now consider an interaction with a finite width by numerically solving the full Eliashberg equations for an e-ph coupling constant g (q) = g0 exp (— |q\/q0). Figure 1 shows the superconducting gap at the lowest Matsubara frequency A (kF, ip/b) as a function oftemperature for several values of 1m and q0 = 0.1/a.We find that the superconducting Tc is already large for a modest value of 1m and increases approximately linearly with 1m in the weak coupling limit; however, the finite range of the coupling in momentum space reduces the total Tc slightly with respect to the perfect forward scattering limit (see the inset of figure 1). The linear dependence of Tc with respect to 1m may account for the wide variation of reported Tc values in the literature, as differences in sample preparation or doping are likely to result in differences in the screening of the e-ph coupling and subsequently Tc.

40 60 80 100 120 T[K]

Figure 1. The superconducting gap at the smallest Matsubara frequency A (ip/b ) as a function of temperature for various values of the e-ph coupling strength Am, as indicated. The e-ph coupling constant g (q) is strongly peaked in the forward scattering direction with q0 = 0.1/a. The inset shows Tc as a function of Am, which is extracted from the data in the main panel. The thin dashed line is the result in the limit of perfect forward scattering (see text). The shaded area represents the values of Am that are relevant for FeSe / STO (see supplementary material6).

T = 100 K

-10 1-10 1 Momentum along (k, 0) [1/a]

Figure 2. The temperature dependence of the spectral function for several values of the e-ph coupling Am.

3.1. Replica bands

The above results show that, in principle, a modest coupling to a phonon with a forward scattering peak is capable of accounting for the large Tc enhancement observed in FeSe on STO and BTO. The natural question is then how much of the experimental Tc is accounted for by this coupling? The observed shape and intensity of the replica bands [7,8] provide us with a direct means to estimate this by comparing our model to experiment. To do so, we calculate the single particle spectral function A (k, w) = —Im G11 (k, w)/p, which requires the analytic continuation of the self-energy to the real frequency axis using the method of [41] (see also supplementary material6). Figure 2 plots the temperature evolution ofthe spectral function obtained from a full numerical solution to our model for several values of 1m, as indicated on the left, and q0 = 0.1/a. In all cases clear replica bands are produced by the coupling, offset in energy from the main band by a fixed energy, which is O for small values of 1m. The separation, however, grows for increasing 1m. This is due to c (k, w), which shifts the main band upward in energy. This is most clearly seen in the 1m = 0.33 results, where the value of kF has visibly shrunk in the main band. In addition, for stronger values of 1m we begin to see the formation of a second replica band located at ~2 W below the main band. Thus the observation of only a single replica band in the bandstructure of FeSe/STO is consistent with a small 1m.

An intuitive picture for the intensity and energy splitting of the replica band can again be obtained in the limit of perfect forward scattering. On the real axis, the zero-temperature self-consistent equation for the self-

Figure 3. The spectral function for a momentum at the band bottom (k = 0 in our model, the Mpoint in the experiment) for T = 30 K, q0 = 0.1/a and Am = 0.02 — 0.22. The key feature of the forward scattering mechanism is the appearance of the mirror band (Z—) next to the main band (Z+). The relative separation Aw andintensity Z—/Z+ = A (0, w—)/A (0, w+) ofthese two features is shown in the inset, and increases approximately linearly with Am. The dashed lines show the corresponding result in the perfect forward scattering limit and the shaded area represents the values of Am that are relevant for FeSe/STO (see supplementary materials6).

qo = 0.1 /a qo = 0.3/a qo = 2/a

Momentum along (A;, 0) [1 /a]

Figure 4. The spectral density A (k, w) along the k = (k/a, 0) cut for q0 = 0.1 (left), 0.3 (middle), and 2 (right). In all three panels the temperature is T = 30 Kand Am = 0.14,0.125, and 0.25 in the left, middle, and right panels, respectively.

energy in the normal state can be written as S (w) = g02 G (w + W).For ^ 0 , the lowest-order solution

is S (w) = + w (note that the ^ 0 solution can be obtained by shifting the self-energy S (k, w) =

S (w — £k)). The poles ofthe Green's function are at w = S (w), which has the solution w± = — W ±

T r qs i n—1

(w±+n>2

W2 + 4g02 .The spectral weight of each pole is given by Z± = — |w=w±J

For small 1m = g02/W2, we find that the average energy separation between the poles is Aw = W [1 + 21m + O (Aim)] and the ratio ofthe spectral weight is ^^ = 1m + O (Aim), thus providing a direct measure of Am.

The spectral weight ratio and energy splitting between the main and replica bands can be extracted from our numerical simulations for finite values of q0. Figure 3 shows A (k, w) for k = (0, 0) as a function of Am with q0 = 0.1/a. The behavior matches our expectations gained from the perfect forward scattering limit: both the distance between the bands and the relative spectral weight grow with increasing Am, though the rate of increase is slower than for the case of perfect forward scattering. ARPES experiments on the FeSe/STO system [7] observe a spectral weight ratio of ~ 0.15-0.2 (see supplementary material6). Comparing to our model calculations, we extract a value of Am ~ 0.15 — 0.2. This corresponds to a Tc ~ 60 — 70 K and a gap magnitude of A ~ 10 — 15 meV, which are consistent with measurements [1,7,10,18].

In figure 4 we present the evolution of the spectral function for increasing values of q0 where Am is fixed to give the same value of Z—/Z+. As expected, the replica bands are observed to smear both in energy and momentum as the value of q0 is increased. This shows that a weakly momentum-dependent coupling (large q0) to an optical mode does not reproduce the observation of a perfect replica band, with the same effective mass and

termination points in the Brillouin zone. Consequently, strong forward scattering is a necessary ingredient to understand the experimental observations [7].

4. Discussion

We have examined the consequences of an e-ph coupling that is strongly peaked in the forward scattering direction on the spectral properties and superconducting transition of a two-dimensional electronic system. We demonstrated that such a coupling produces distinct replica bands in the electronic bandstructure consistent with recent ARPES measurements on FeSe/STO and FeSe/BTO interface systems. In order to reproduce the experimentally observed spectral function, we find that relatively modest values of the e-ph coupling are needed with 1m ~ 0.15 — 0.2. Strong forward scattering results in a momentum decoupling of the Eliashberg equations, which subsequently produces a larger superconducting Tc in comparison to the predictions of conventional BCS theory. As a result, the inferred values of 1m predict Tc values on the order of60-70 K due to e-ph coupling alone.

We stress that our results do not exclude the presence of another unconventional pairing channel such as spin fluctuations. The predicted values of Tc and A will be reduced somewhat by the inclusion of the Coulomb pseudopotential m*. (For example, we examined the influence of m* and found that Tc is lowered by ~20% for m* ~ 0.2 (see supplementary material6). This is much smaller than the factor of 2-5 commonly obtained for conventional phonon-mediated pairing [42,43]. This robustness is linked to the same momentum decoupling responsible for the linear dependence of Tc on Am.) This reduction, however, can be overcome by the combination of the e-ph and unconventional interactions, since forward scattering will contribute to Cooper pairing in most channels [7]. An obvious way to distinguish between these possible scenarios is to measure the oxygen isotope effect. If a purely phononic mechanism is present then Tc should have an isotope coefficient a = — 9 log (Tc)/9 log (M) = 1/2,whiletheenergyseparationbetweenthereplicabandsshoulddecreaseby ~0.5 (18 — 16^ 16 ~ 6% for 18O rich substrates. Alternatively, in a multi-channel scenario, the isotope coefficient a will be reduced from 1 /2 when the unconventional channel is significant in comparison to the e-ph interaction [38-40]. This provides a clear means to distinguish between these scenarios.

Finally, we note that e-ph coupling with a pronounced forward scattering peak has been studied in several contexts related to of unconventional superconductivity in the cuprates [24-30] andpnictides [31]. Moreover, it is also now being addressed in the context of nematic fluctuations [44,45]. This suggests forward scattering has a broader applicability in enhancing superconducting beyond interface systems.

Acknowledgments

We thank E Dagotto, T P Devereaux, D-H Lee, R G Moore, and J Zaanen for useful discussions. LR acknowledges funding from the Dutch Science Foundation (NWO) via a Rubicon Fellowship. TB is supported as a Wigner Fellow at the Oak Ridge National Laboratory. A portion of this research was conducted at the Center for Nanophase Materials Sciences, which is a DOE Office of Science User Facility. CPU time was provided in part by resources supported by the University of Tennessee and Oak Ridge National Laboratory Joint Institute for Computational Sciences (http://jics.utk.edu).

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