Almost a decade has passed since the serendipitous discovery of the iron-based high temperature superconductors (FeSCs) in 2008. The fact that, as in the copper oxide high temperature superconductors, long-range antiferromagnetism in the FeSCs arises in proximity to superconductivity immediately raised the question of the degree of similarity between the two. Despite the great resemblance in their phase diagrams, there exist important differences between the FeSCs and the cuprates that need to be considered in order to paint a full picture of these two families of high temperature superconductors. One of the key differences is the multi-orbital multi-band nature of the FeSCs, which contrasts with the effective single-band nature of the cuprates. Systematic studies of orbital related phenomena in FeSCs have been largely lacking. In this review, we summarize angle-resolved photoemission spectroscopy (ARPES) measurements across various FeSC families that have been reported in literature, focusing on the systematic trends of orbital dependent electron correlations and the role of different Fe 3d orbitals in driving the nematic transition, the spin-density-wave transition, and superconductivity.
Thirty years after the historic discovery of cuprate high temperature superconductors, the mechanism for high temperature superconductivity remains the biggest challenge in condensed matter physics despite tremendous amount of theoretical and experimental efforts. The discovery of iron-based superconductors1 provides a great opportunity to identify the important ingredients that are common to both families of high Tc materials and to test the theoretical models that have been formulated for cuprates. Comparing FeSCs with cuprates, the most striking similarity is the common phase diagram, in which unconventional superconductivity appears in the vicinity of other competing phases, such as the pseudogap phase and the charge order in cuprates and the spin-density-wave (SDW) phase and nematic phase in FeSCs.2,3 The emergence of superconductivity always takes place with the suppression of these competing phases. Such a remarkable resemblance has raised our hope for a unified theory of high temperature superconductivity and has motivated many theorists to take the strong coupling approach to describe FeSCs.
On the other hand, FeSCs also appear to distinguish themselves from cuprates in various aspects, including metallicity of the parent phase, crystal structure of the conduction layer, spin symmetry of the antiferromagnetic order, as well as the underlying electronic structure. Prior to establishing a unified understanding of the physics in cuprates and FeSCs, we first need to understand whether these differences are trivial nuances or critical ingredients that cannot be neglected. Among them, the most fundamental difference is the multi-orbital multi-band nature of the underlying electronic structure in FeSCs. In contrast to cuprates, for which essential physics seems to take place in a single effective band and Fermi surface, there are at least three out of five Fe 3d orbitals that are active near the Fermi level (E F) in FeSCs, forming multiple Fermi surface sheets. The complexity of theoretical treatment for a multi-band system has led to various proposals for minimal models for FeSCs, in which the orbital degree of freedom is often ignored for simplicity. While these models capture some underlying physics, the question is whether they miss important orbital related physics.
The lack of systematic experimental studies on the role of different Fe 3d orbitals may be part of the reason that orbital physics in FeSCs has not garnered as much attention as they perhaps deserved. In this review, we summarize experimental evidence of various orbital dependent phenomena in the electronic structure from angle-resolved photoemission spectroscopy literature. For a recent review on the progress of theoretical studies on the orbital degree of freedom, please see ref. 4. First, we discuss systematic trends on the normal state electronic structure across different families of FeSCs. In particular, we point out a systematic change of the orbital related physics, for example the increase of orbital-selective electron correlations across the wide spectrum of FeSC compounds based on both structural parameters and charge carrier doping. Eventually, this growth of orbital-dependent correlations naturally culminates in a complete localization of a single orbital while other orbitals remain itinerant—an orbital-selective Mott phase. Hence the orbital degree of freedom plays an important role in balancing the coexistence of local and itinerant physics in the normal state of the FeSCs. We then focus on the manifestations of different Fe 3d orbitals across the nematic and the SDW transitions. In the nematic state, strong anisotropy occurs in the hopping of the dxz, dyz, and dxy orbitals as characterized by a momentum dependent reconstruction of dxz, dyz, and dxy bands. In the SDW state, bands fold and SDW gaps open. The SDW gap is also strongly orbital-dependent. It is large on the dxy bands but moderate on the dxz/dyz bands. These observations have strong implications on the theories aiming to understand the nature of those competing phases and suggest an important role of multi-orbital nature of FeSCs in driving the nematic and SDW transitions. In the end, we discuss the non-trivial implications of multi-orbital nature on the superconducting pairing mechanism of these materials.
The normal state
All FeSC compounds, regardless of their compositions, share in common planes containing iron and pnictogen (P/As) or chalcogen (S/Se/Te), which is located alternatingly above and below the Fe lattice (Fig. 1a). The difference among FeSC families is the composition and structure of interlayers between the Fe planes. In some cases, these interlayers form charge reservoirs that donate charge carriers to the Fe planes. The normal state is defined as the phase outside the boundaries of the magnetic and structural transitions (Fig. 1a). All FeSC compounds share in common the basic electronic structure consisting of Fe 3d bands near E F, with the dxz, dyz, and dxy orbitals most active near E F. The basic electronic structure of FeSC in the normal state is illustrated in Fig. 1c, where three hole-like bands reside near the Brillouin Zone (BZ) center, Γ, and two electron-like bands near the BZ corner, M (except in the case of the 122 structure, where this point is called the X point). For different doping levels and structural subtleties, the overall or relative positions of the hole and electrons bands may vary in energy, leading to different Fermi surface topologies with varying number of hole pockets at Γ and electron pockets at M (Fig. 1d). For undoped parent compounds, the hole pockets at Γ and electron pockets at M are of similar sizes. For hole-doped compounds, the hole pockets at Γ enlarge while the electron pockets shrink. For heavily electron-doped compounds such as the electron-doped chalcogenides, the hole pockets disappear while large electron pockets remain at M.
One of the fundamental questions after the discovery of the FeSCs was whether it is appropriate to model them as localized systems or itinerant systems. On one hand, the observed large spectral weight in the fluctuating magnetic spectrum5 tends to suggest the former, while the high density of states found near E F compared to the cuprates6 seems to suggest the latter. As we know now, neither picture is fully complete. We will show in the following that there is a large systematic spread of electron correlation strength among different FeSCs, and more importantly, this occurs in a strongly orbital-dependent way.
This trend can be qualitatively seen by comparing representative compounds from the iron phosphides to the iron arsenides and to the iron chalcogenides (Fig. 2). Electron correlation renormalizes the electronic bandwidth. From ARPES data, one way to quantify the strength of correlation is to extract the ratio of the non-interacting bandwidth calculated from local density approximation (LDA) and experimentally measured bandwidth, which is the renormalization factor.7 Figure 2a–c shows the band dispersions along the high symmetry direction Γ–M observed in the paramagnetic state of a phosphide (SrFe2P2), an arsenide (NaFeAs), and a chalcogenide (FeSe0.44Te0.56), plotted in the same energy window, where the dyz band is marked in green and dxy blue. There are two observations to make: (i) the bandwidth of all bands systematically narrows from phosphide to the arsenide to the chalcogenide, which is also seen in the increase of the renormalization factors, and (ii) the bandwidth of dxy narrows at a much faster rate than that of dyz from the phosphides to the chalcogenides. These two observations suggest that both the overall electron correlation strength and orbital-selectivity, which is defined here as the ratio in the band renormalization between the dxy band and dyz band, increase from the iron phosphides to the iron chalcogenides. In the following section, we systematically demonstrate these trends and discuss factors that correlate with these two parameters.
Considering the three active orbitals near E F, the dxz and dyz orbitals are bound by C4 symmetry to be degenerate in the tetragonal state. The dxy orbital, however, does not necessarily need to behave in the same way as dxz/dyz. Hence we examine each orbital in turn. For the bands near E F, the dyz band is the band that can be observed most completely under common polarization setups, with its band top at Γ and band bottom between Γ and M (Fig. 1c). Here we extract its bandwidth from ARPES literature and compare with available LDA calculations (Table 1). Figure 2d shows the dyz renormalization factors for FeSC compounds measured in the normal state as a function of the Fe-Pn/Ch bond length. To avoid complications from doping effects, we only plot undoped parent compounds here where the electron filling, n, is 6. First of all, we see a clear trend with a continuous spread of renormalization factors from the phosphides at the bottom to the 122 arsenides to the 111 arsenides and to the chalcogenides. The dyz renormalization factor, which is a measure of overall correlation strength, increases with the Fe-Pn/Ch bond length. Intuitively, longer bond length reduces electron hopping and therefore the kinetic energy, hence leading to more localized behavior. However, similar plot for the dyz and dxy renormalizations as a function of the lattice a (effectively Fe-Fe bond length) does not show as clear a trend over all compounds (Fig. 3a, c). As dyz is extended in the out-of-plane direction and dxy is mostly in plane, the lack of clear trend in both renormalizations against lattice a suggests that electron hopping is dominated by the indirect path of Fe–Pn/Ch–Fe rather than that of direct Fe–Fe bond. The dyz renormalization factor also has strong correlation with related structural parameters such as anion height and bond angle, which both directly relate to the Fe–Pn/Ch bond length.8 Similar dependence of correlation strength on structural parameters is also seen in optical data within the BaFe2As2 family9 and photoemission data within the heavily electron-doped iron chalcogenides.10 For other structural parameters such as the lattice constant c, the correlation with bandwidth renormalization is not obvious across families (Fig. 3b, d).
Structural parameters are not the only factors that correlate with the overall correlation strength. A second factor is electron filling.7 In Fig. 2e we plot the dyz bandwidth renormalization vs. the electron filling for doped compounds of two series, the BaFe2As2 series and the LiFeAs series. To put this plot in perspective, we also overlay the electron (Co) and hole (K) doped phase diagram of BaFe2As2 on the horizontal axis. The data points for this series range from those taken from KFe2As2 (n = 5.5) to BaNi2As2 (n = 8). Here we note that the undoped parent compounds of FeSC has n = 6, which is not half-filling as the case of the parent compounds of the cuprates. True half-filling for the Fe 3d orbitals is n = 5. This explains the asymmetry of the overall correlation with respect to the undoped parent compounds of FeSC.7,9 The electron correlation is weak far away from n = 5 for the heavily electron-doped compounds, and diverges towards n = 5 on the hole-doped side. However, it is interesting to note that, under this scenario, the known undoped iron pnictides are effectively on the electron-doped side of the true half filling. In analogy to the cuprates, there may be an equivalent regime of superconductivity on the hole-doped side, as has been recently theoretically suggested.11,12
In Fig. 2f we plot all the compounds (including those with different electron fillings) with sufficient information from literature on a 2D plot with electron filling and the Fe–Pn/Ch bond length, and use color to indicate the strength of dyz bandwidth renormalization factor. Here we see as demonstrated before, both reducing electron filling towards n = 5 and lengthening the Fe–Pn/Ch bond length increase overall correlation.
Next, we discuss factors that affect the orbital-selectivity. Since the dxy orbital is the most correlated of the orbitals, quantitatively, we extract the ratio of the renormalization factors of the dxy band and the dyz band. In Fig. 2h we plot this for all compounds we found from literature against the Pn/Ch–Fe–Pn/Ch bond angle. A clear trend is seen where smaller bond angle, as in the case of the chalcogenides, leads to strong selectivity; whereas bigger bond angle, as in the case of the phosphides, leads to almost no selectivity. This is because smaller bond angle results in a vertically elongated tetrahedron, which reduces hopping more dramatically for the in-plane dxy orbital than dxz/dyz orbitals, considering hopping is dominantly mediated through the Pn/Ch, which reside out of the Fe plane. Besides the bond angle, Fig. 2g also shows another factor that correlates with orbital-selective correlation—the overall electron correlation represented by the dyz renormalization factor. It demonstrates that among all FeSCs, the stronger the overall correlation, the stronger the orbital-selectivity in the dxy orbital. This has been discussed in previous theoretical work as due to the tendency towards a Hund’s metal phase, where Hund’s coupling increases orbital differentiation and independence by suppressing inter-orbital correlations.8,13,14 In Fig. 2i, we plot the orbital-selectivity as a function of both bond angle and overall correlation strength for all compounds. We see that these dependences are not only true within a family of FeSC, but systematically spread among all FeSC compounds.
As orbital-selectivity increases, an interesting phenomenon occurs in the strongly correlated members of FeSCs—a tendency towards an orbital-selective Mott phase (OSMP). In Fig. 4a, we plot the bond length dependence of the renormalizaton factors of the dxy orbital for undoped FeSCs (n = 6), which is the most correlated orbital. Comparing to the equivalent plot for dyz (Fig. 2d), we see that the dynamic range of the dxy orbital is five-fold of that of dyz. This again showcases the strong orbital differentiation among the FeSCs towards the strongly correlated members. When this differentiation is strong, as in the iron chalcogenides, the normal state of these materials is sufficiently close to an OSMP such that raising temperature has been observed to push them into the OSMP where the dxy orbital completely loses its spectral weight while other orbitals remain itinerant.15 This has in fact been observed universally for different iron chalcogenides including Fe(Te,Se), KFe2Se2, and monolayer FeSe film grown on SrTiO3 16,17,18,19 (Fig. 4b) and Nb:BaTiO3/KTaO3 heterostructures.20 Even for the most correlated iron arsenide, KFe2As2, evidence for decoherence of the dxy orbital has been observed by transport measurements.21 Here we see that the tendency towards the OSMP in the chalcogenides is not accidental, but grows naturally from an increasingly selective orbital correlation systematically in all FeSCs.
Both the spread of electron correlation strength and the increasing orbital selectivity are perhaps what makes it difficult to develop a unified theoretical model for all FeSCs. On one side of the spectrum the orbitals are mostly itinerant with almost no orbital selectivity while on the other side strong orbital decoupling due to Hund’s coupling results in one of the orbitals approaching localization. Nonetheless, this orbital-selectivity is a behavior unique and essential to the multi-orbital physics of the FeSCs in contrast to the single-band physics of the cuprates. Its importance is especially evident for the compounds on the strongly correlated side such as the chalcogenides. These behaviors have led to interesting theoretical proposals where one redefines the phase diagram using an average orbital filling, showing a gradual approach from superconductivity towards a Mott insulating state via an OSMP,13 while another proposes that in the strongly orbital-selective regime, the dxy orbital is near half-filling.14 Both suggest parallels reminiscent of the cuprate problem.
The nematic state
In a typical phase diagram of iron-based superconductors, the material in the underdoped regime goes through two transitions and enters the nematic state and the SDW state at low temperatures.2,3 The multi-orbital nature not only leads to orbital-dependent band renormalization in the normal state, but also plays an important role in driving the system into these symmetry-breaking states. The nematic phase is marked by a tetragonal to orthorhombic structural transition at TS, where C4 rotational symmetry is broken down to C2 symmetry without breaking the translational symmetry. With the orthorhombic distortion, material forms natural twin domains. Hence for macroscopic probe like ARPES where the beam spot is larger than the typical domain size (Fig. 5a), the photoemission signal becomes the superposition of band structures from two orthogonal domains. As a result, complex band reconstructions were reported in early ARPES studies.22,23,24 Subsequently, it was realized that samples with a single domain could be achieved by applying a uniaxial pressure mechanically on the sample.25,26 The intrinsic band structure of the C2 state was then revealed by ARPES measurements on detwinned crystals of BaFe2As2,27,28,29 NaFeAs,30,31 and FeSe,32,33, and inferred thereafter from twinned crystals of FeSe34,35 and FeSe films.36,37 Figure 5b shows an example of detwinned NaFeAs measured in the nematic state, where the dyz band (green) along the slightly longer axis is shifted up while the dxz band (red) along the shorter axis is shifted down. In the tetragonal state above TS, these two bands are degenerate in energy. This shift in opposite directions in the orthorhombic state indicates the breaking of the C4 symmetry in the orbital degree of freedom. This generic upward shift of dyz orbital and downward shift of dxz orbital is observed in all measurements of FeSCs in the nematic phase.27,28,29,30,31,32,33,34,35,36,37 Importantly, the relatively large energy scale of this orbital splitting cannot be a trivial consequence of the less than 1% orthorhombicity.27 Hence the orbital anisotropy is unlikely to be a simple result of the lattice, but rather suggests the manifestation of electronic nematicity, consistent with the original discovery of large resistivity anisotropy in this phase.25 We note that, on top of the discussed band separation, an additional small band splitting has been observed by ARPES in FeSe,38,39 which induced hot debates on how to extract the correct nematic energy splitting from the ARPES data. The energy scale of the large band separation scales with the nematic transition temperature in all measured FeSCs and thus likely represents the strength of nematic order. Moreover, very recent data on detwinned FeSe clearly shows the two bands with large energy separation to belong to orthogonal directions,40 hence consistent with the previous understanding that the dxz and dyz orbitals are indeed split by ~50 meV in the nematic phase, similar to the pnictides.
The discovery of energy splitting of dxz and dyz bands has been viewed as an evidence for the existence of orbital order in the nematic state. It has been proposed that the on-site occupation difference between dxz and dyz orbitals triggers a ferro-orbital ordering, which consequently drives the system into the nematic state.41,42,43 In most band calculations where only the on-site occupation difference is considered, the ferro-orbital order results in an energy splitting of dxz and dyz bands that is almost constant throughout the BZ. Experimentally, clear delineation of the momentum dependence of the dxz and dyz splitting has not been carefully examined for most FeSCs, because the close proximity of the magnetic and structural transitions prevents a clear separation of the effects of the two phases. FeSe, which does not have a magnetic transition,44 offers a clean case for examining the nature of nematic order and associated nematic transition in detail. Figure 5c shows the band dispersions along the high symmetry direction Γ–M of a twinned multi-layer FeSe film grown on SrTiO3,36 which resembles bulk FeSe crystal. On a twinned sample, the longer and shorter orthogonal high symmetry directions from orthogonal domains are superpositioned along the same cut. Hence the shifted dxz/dyz bands appear as effectively split in energy below TS. From this data, two important observations can be made. Firstly, the dxz/dyz bands, which are degenerate above TS, are split in the same fashion as in other FeSCs. Secondly, a clear momentum-dependence is seen in this orbital anisotropy. As shown in Fig. 5d, instead of being constant, a finite energy splitting at Γ first decreases to zero and then increases again, reaching its maximum at the M point. The momentum-dependence of the energy splitting is consistent with BaFe2As2 and NaFeAs, where the orbital anisotropy is small at Γ but large at M27. Furthermore, the momentum dependence of orbital anisotropy is non-monotonic, which may be understood by considering a band splitting (Eyz−Exz) that switches sign between Γ and M (Fig. 5e). This has indeed been experimentally observed in detwinned FeSe bulk crystal.35,40 This non-trivial momentum dependence of the dxz/dyz energy splitting suggests that the simple on-site occupation difference between dxz/dyz orbitals is unlikely to be the driving force of the nematic phase. Instead, other mechanisms such as anisotropic hopping of the dxz/dyz orbitals,45,46 Pomeranchuk instability,47 orbital-dependent correlation effect,48 and orbital-selective spin fluctuations49 could all result in different renormalization and/or shift of the dxz/dyz bands in the nematic state.
While the dxz/dyz orbital anisotropy has attracted great attentions, the dxy orbital has not been considered in most theoretical models, partly due to the lack of experimental evidence for a clear participation of dxy orbital in the electronic reconstructions and the assumption that it does not contribute to C4 symmetry breaking. However, as illustrated in Fig. 5f and g, to fully explain the three electron bands observed in the nematic phase at the M point on this twinned sample, the shift of the dyz and dxz bands in opposite directions is insufficient, in addition, the dxy band along the longer x-direction must shift down in energy while the counterpart dxy band along the shorter y-direction must remain unshifted.36 Furthermore, the magnitude of the energy splitting of the dxy band along two perpendicular directions is comparable to the energy splitting of the dxz/dyz orbitals, which further suggests the complexity of the orbital anisotropy in the nematic state.
The observed band reconstruction and its orbital dependence put strong constraints on theoretical models regarding the nematic state. On one hand, while most theories consider only the dxz/dyz orbitals, the ARPES results suggest that all three orbitals play an important role in driving the nematic state. As one theoretical study shows, the coupling of the dxy orbital to the nematic order parameter is necessary for predicting the correct gap symmetry in FeSe.50 On the other hand, the energy scale of the band reconstruction shows a strong momentum dependence, indicating that the anisotropy is unlikely to be dominated by the on-site occupation difference between the dxz and dyz orbitals. Instead, other mechanisms must be considered to correctly describe the momentum-dependence orbital anisotropy.
The spin-density wave order
Next, we discuss the role of different orbitals in forming the collinear SDW order. The SDW order has been found to couple strongly with the nematic order in most cases. On top of the rotational symmetry breaking, the SDW order further breaks the translational symmetry. As a result, the BZ reduces and bands fold across the SDW zone boundary. Spectrally, the signatures of the SDW band reconstruction are very distinct from that of the nematic phase. Instead of the band shift, SDW gaps open where folded bands cross original bands. It is simpler to illustrate the details of the band folding by unfolding the bands into the 1-Fe BZ, where the folding occurs strictly along the AFM direction Γ−M x but not along the FM direction (Fig. 6a). Here, the Γ point has two hole pockets from the dxz and dyz hole bands. At the M x point, an electron pocket appears that is of dxy character along the AFM direction and dyz along the FM direction. At the M y point, another electron pocket appears with dxy along the FM direction and dxz along the AFM direction. At the Γ‘ point, in some of the iron-arsenide compounds, lives the third hole pocket of dxy character. With SDW folding, the Γ and Mx points fold unto each other, while the M y and Γ‘ points fold unto each other.
Next, we discuss the detailed band reconstruction around these two folded points using data from detwinned BaFe2As2, which can be revealed by using different polarizations. For the folded Γ–Mx cut (Fig. 6b), along the AFM direction, the dxy electron band from Mx folds unto the dxz and dyz hole bands around Γ, but little or no SDW gap appears along this high symmetry direction where folded bands cross. Along the orthogonal FM direction at this same point (Fig. 6c), the dyz electron band crosses the dxz/dyz bands, forming an SDW gap on the order of ~30 meV between the dyz bands, which can be seen in both the dyz hole band and the dyz electron band. For the folded My–Γ‘ point (Fig. 6d), along the AFM direction, the dxz electron band crosses the dxy hole band, opening an SDW gap that saddles E F, with a gap size bigger than 50 meV. Along the orthogonal FM direction at this point (Fig. 6e), the dxy hole and electron bands cross each other, opening an SDW gap that is larger than 50 meV. Overall, we see that the SDW gap opens at the folded band crossings in an orbital-dependent way. The biggest SDW gaps occur in the dxy bands around the M y–Γ‘ point. The SDW gap is moderate for the dyz bands at the Γ–Mx. For the dxz hole bands, the SDW gap is the smallest, resulting in dominant dxz orbital weight near the Fermi energy in the SDW state.51 Four SDW gap nodes exist along the high symmetric directions due to the incompatible symmetries of the crossing bands.52 As a result, the Fermi surface reconstructs drastically, forming four small Fermi pockets along both the Γ–Mx and Γ–My directions (lower panel of Fig. 6a).
The SDW order has been described in both weak-couplings and strong-coupling theories. It is still largely debated whether the SDW is originated from the super-exchange interaction of local moments or the Fermi surface nesting of itinerant electrons.5,53,54,55,56,57,58 The orbital-dependence of the band reconstruction in the SDW state suggests an orbital-selective magnetism in the iron-based superconductors. It has been proposed that the magnetic moments originate mainly from the dxy and dyz orbitals instead of the dxz orbital in the SDW state,59,60,61 which is consistent with the orbital-dependent SDW gaps observed here. The multi-orbital nature of the SDW state also explains the dual character of the magnetic moments observed by neutron scattering experiment.53 Both the local property of dxy orbital and the itinerancy of the dyz/dxz orbitals should be considered in constructing the microscopic model of the SDW state in iron-based superconductors.
The superconducting state
Finally, we discuss the role of orbitals in the superconducting state. While the superconducting gap in cuprates can be fitted by a simple dx2−y2 gap function across all different families, the gap symmetry in FeSCs has a complex distribution in momentum space that varies among different families:62 while largely isotropic gaps have been observed in Ba1−xKxFe2As2 62 consistent with s± symmetry, strong gap anisotropy or even gap nodes have been reported in BaFe2(As1−xPx)2,63,64 LiFeP,65 bulk FeSe,66 FeSe1−xSx,67 and FeSe films.68 In cases like 1 mL FeSe thin film, the gap function cannot be fitted by single trigonometric gap functions under s±, d-wave, or extended s-wave gap symmetries.69 This contrasting behavior is intimately connected to the multi-band multi-orbital nature of the underlying electronic structure and again implies the non-trivial role which orbital physics plays in the FeSCs.
Frist of all, the Fermi surface of FeSCs consists of multiple Fermi pockets with distinctive orbital characters. Such Fermi surface topology allows Cooper pairs to scatter via intra-orbital or inter-orbital scattering channels. One critical question is which scattering channel is more important for superconducting pairing. The intra-orbital pairing would result in an orbital dependent superconducting gap while the inter-orbital pairing tends to generate equivalent gaps among different orbitals. Experimentally, multi-gap behavior has been observed in several iron-based compounds by scanning tunneling microscopy (STM)70,71 and transport measurements.72,73 ARPES studies on Ba1−xKxFe2As2 and LiFeAs show that the superconducting gap on the dxz/dyz hole pockets is much larger than that on the dxy hole pocket.62 All these results seem to suggest the dominating role of intra-orbital pairing in FeSCs.
Another important question often asked is which orbital plays the most important role for superconductivity. This, too, seems to vary between different compounds. For most iron-pnictide compounds studied with comparable hole and electron pockets, the dxz/dyz hole pockets show larger superconducting gap than the dxy hole pocket,62,74 suggesting the importance of dxz/dyz orbitals to superconductivity. Consistently, in LiFe1−xCoxAs and Ba(Fe1−xCox)2As2, when the dxz/dyz hole pockets vanish with electron doping, superconductivity is strongly suppressed.75,76 On the contrary, for heavily electron-doped iron-selenide superconductors with only electron pockets, the superconducting gap of 1 mL FeSe film show maxima on the dxy electron bands.69 Furthermore, in bulk FeSe crystal, where the sample is continuously surface-doped to enhance superconductivity, it is reported that the appearance of the dxy electron pocket on the Fermi surface at the M point coincides with the beginning of the second superconducting dome with higher TC and different pairing symmetry.77 Interestingly, another work on the pnictide compound Ca10(Pt4As8)(Fe2−xPtxAs2)5 shows relatively high TC with the presence of only the dxy hole pocket at Γ.78 This may on one hand suggest the importance of the dxy orbital to superconductivity, on the other hand highlight the strong correlation between inter-pocket (intra-orbital) scattering and superconductivity.
The level of material-dependence reported in the past decade has been somewhat puzzling and perhaps disappointing for the ultimate goal of finding a simple unifying description of superconductivity. However, this may be well expected when we consider the multi-orbital nature of the FeSCs. As this is a new dimension which has been lacking from the machinery developed out of the cuprate problem, theoretical work taking into account the orbital degree of freedom has been very limited, but several work have already showed promise. From the strong coupling approach using a multiorbital t–J 1 –J 2 model, one study showed that the orbital-selectivity results in a gap anisotropy that is also orbital-dependent.79 From a weak-coupling approach, a very recent theoretical study based on spin fluctuations taking into consideration the orbital-selective renormalization that modulates the coherent spectral weight of different orbitals was able to reproduce the observed momentum-dependent gap structure of monolayer FeSe and LiFeAs.80 Other theoretical works have also proposed interesting mechanisms by which the FeSCs and cuprates could be united.81,82 These work importantly demonstrate that behind the apparent gap variations amongst FeSCs there may be a common underlying pairing mechanism, and the source of the material-dependence may be the different degree of orbital-selective correlation effects, which tune the dominant orbitals that are manifested.
We first summarize the key findings of the four major phases discussed:
The normal state:
Electron correlations systematically and continuously spread across FeSC families tuned by two factors: i) the Fe–Pn/Ch bond length, and ii) electron doping away from true half-filling at n = 5.
Electron correlations are orbital-dependent, with the dxy orbital being the most localized. The strength of orbital-selectivity is tuned by i) overall correlation strength, and ii) bond angle, eventually reaching an orbital-selective Mott phase where the dxy orbital is completely localized while other orbitals remain itinerant.
The nematic state:
There is significant C4 symmetry breaking in the orbital degree of freedom at the onset of the structural transition beyond the effect of the lattice distortion. In particular, the dyz-dominant band is observed to shift up while the dxz-dominated band is observed to shift down, albeit in a strongly-momentum dependent way.
The dxy orbital is also observed to participate by exhibiting a splitting in energy that is comparable to that of dxz/dyz orbitals, suggesting an anisotropic hopping origin rather than ferro-orbital order.
The spin density wave order:
Band folding occurs, producing SDW gaps that are the largest in the dxy orbital, moderate in the dyz orbital, and smallest in the dxz orbital.
The superconducting state:
Superconducting gaps are generally observed to be multi-gap, suggesting dominance of intra-orbital pairing.
Gap functions cannot be described by single trigonometric gap functions, and also vary among families, suggesting the complex role of intra-orbital pairing and multi-orbital FS.
Having discussed the normal state, the nematic state, the magnetic state, and the superconducting state separately, we now discuss the relationship between these phases. From the normal state properties, we see that there is a systematic spread of electronic correlation over all the FeSCs, with a large dependence on certain structural parameters such as the bond length and bond angle. As has been shown, the superconducting temperature, TC, is also highly dependent on the bond angle.83 Hence superconductivity is expected to be optimized at intermediate electron correlation strength. The nematic phase and the collinear SDW phase are often discussed together. Here we see that the two orders can be strongly coupled, as in most iron arsenides, but not necessarily always the case, as in FeSe. Regardless of the strength of coupling of these two orders, we see that the spectral signature and magnitude for the nematic order is the same across different materials. The nature of these two phases to superconductivity is competitive. As has been reported, the spectral order parameters of these two orders both decrease at the onset of superconductivity,84 similar to the macroscopic order parameters of the lattice orthorhombicity and the magnetic moment.85
For all three phases discussed, we also see a strong orbital-dependence. Hund’s coupling suppresses orbital interaction, separating the dxy orbital from the largely degenerate dxz/dyz. This coupled with crystal field splitting effectively makes the dxy orbital the most strongly correlated, as seen in the normal state, and in some cases close to half-filling while the overall filling is effectively on the electron-doped side. This occurrence enables some behaviors of the dxy orbital in the FeSCs to become relevant to the cuprates, such as the observation of OSMP in the most correlated iron chalcogenides. We have also seen that the dxy orbital actively participates in the nematic and magnetic competing phases to superconductivity, by both developing a non-trivial anisotropy below TS and the largest SDW gap below TSDW. The dxz/dyz orbitals, on the other hand, are less correlated than dxy and maintains a certain level of itinerancy due to their degeneracy and effective electron-doping away from half-filling. This degeneracy also gives them a more active role in the nematic phase, where the degeneracy is lifted below TS.
Overall, we see that the orbital-dependence in the FeSC plays a nontrivial role. The systematic spread of orbital-selective electron correlations across different FeSC families may well be the origin of material-dependent variations that is manifested when the participation of different orbitals is enhanced or suppressed in different phases. When taken under this perspective, there is still hope that the underlying mechanism for superconductivity and competing phases in the FeSCs and perhaps even the cuprates may take on a unified simple form, upon which the orbital-selective physics adds on an essential and colorful light.86,87,88,89,90,91,92,93,94,95,96,97,98,99,100,101,102,103,104,105,106,107,108,109,110,111,112,113,114,115,116
The data sets used for the normal state properties were taken from available literature and the references are all provided in Table 1.
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The authors would like to thank Véronique Brouet, Thomas Devereaux, Rafael Fernandes, and Leni Bascones for enlightening discussions, and David Singh for kindly providing LDA calculations for SrFe2P2. This work was supported by the U.S. Department of Energy, Office of Science, Basic Energy Sciences, Materials Sciences and Engineering Division under contract DE-AC02-76SF00515. Stanford Synchrotron Radiation Lightsource and the Advanced Light Source are both operated by the U.S. Department of Energy, Office of Science, Office of Basic Energy Sciences.
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Nature Communications (2018)