# Band-dependent superconducting gap in SrFe2(As0.65P0.35)2 studied by angle-resolved photoemission spectroscopy

## Abstract

The isovalent-substituted iron pnictide compound SrFe2(As1−xPx)2 exhibits multiple evidence for nodal superconductivity via various experimental probes, such as the penetration depth, nuclear magnetic resonance and specific heat measurements. The direct identification of the nodal superconducting (SC) gap structure is challenging, partly because the presence of nodes is not protected by symmetry but instead caused by an accidental sign change of the order parameter, and also because of the three-dimensionality of the electronic structure. We have studied the SC gaps of SrFe2(As0.65P0.35)2 in three-dimensional momentum space by synchrotron and laser-based angle-resolved photoemission spectroscopy. The three hole Fermi surfaces (FSs) at the zone center have SC gaps with different magnitudes, whereas the SC gaps of the electron FSs at the zone corner are almost isotropic and kz-independent. As a possible nodal SC gap structure, we propose that the SC gap of the outer hole FS changes sign around the Z-X [(0, 0, 2π) − (π, π, 2π)] direction.

## Introduction

Since the discovery of high-temperature superconductivity in the iron pnictides and chalcogenides1, the mechanism of Cooper pairing and the symmetry of the order parameter have been central issues of debate2,3. In the spin-fluctuation-mediated superconductivity, intra-orbital nesting between hole and electron Fermi surfaces (FSs) brings about a sign-changing s±-wave superconducting (SC) state4,5,6. In the orbital-fluctuation-mediated superconductivity, a sign-preserving s++-wave SC state is expected7,8. In heavily overdoped systems such as Ba1−xKxFe2As2, where the electron FSs at the zone corner are absent or much smaller than the hole FSs at the zone center, a d-wave pairing9 and time-reversal-symmetry-broken pairings such as s + is and s + id symmetries have been proposed10,11. The diversity of the SC gap structure among various materials and doping elements characterizes the FeSCs in comparison with the cuprates12.

Among the FeSCs, the isovalently-substituted BaFe2(As1−xPx)2 (Ba122P) system13 has attracted particular attention since the presence of line nodes in the SC order parameter was proposed from NMR14, penetration depth, and thermal conductivity measurements15. If the symmetry of the order parameter is A1g, line nodes are realized by an accidental crossing of the zero surface of the order parameter and the FSs16, which requires a careful experimental investigation into the location of nodes in the momentum space.

The structure of the accidental node of the SC gap sensitively depends on the microscopic pairing mechanism. In the spin-fluctuation-mediated pairing mechanism, the SCgap tends to change its sign along the nesting vector. In particular, the pnictogen height sensitively controls the radii of FSs and the nesting vectors, thereby switching the nodal and nodeless SC gaps17. Suzuki et al.18 have calculated the three-dimensional SC gap structure within the random phase approximation (RPA) using the lattice parameters of Ba122P, and shown that the SC gap on the outer hole FS around the Z [(0, 0, 2π)] point that has a contribution from the dz2 orbital character is small (below 2 meV) and may change sign. Furthermore, the gap shows in-plane anisotropy with the strongest tendency to sign change along the direction 45° off the Z-X direction. On the other hand, Saito et al.19 have shown that, by taking orbital flucutuations into account, a nodal s-wave state may appear with loop-shaped line nodes on the electron FSs. Furthermore, in stark contrast to the spin-fluctuation scenario, the gap function on the outer hole FS around the Z point may have a finite value that is comparable to those in the other two hole FSs, as a result of the interorbital correlations among the d orbitals.

Given the distinct behavior of the theoretical SC gap expected for different pairing interactions, experimental information about the orbital dependence of the SC gap and the location of line nodes will shed light on the microscopic mechanism of the Cooper pairing. In order to clarify them, the SC gap of Ba122P has been studied using various experimental probes. Shimojima et al.20,21 have found a nearly isotropic, orbital-independent SC gap opening on the three hole FSs around the Z point by high-resolution laser-based angle-resolved photoemission spectroscopy (ARPES). Furthermore, Yamashita et al.22 observed a fourfold oscillation in angle-resolved thermal conductivity as a function of magnetic field direction within the basal plane. They have concluded that loop-like line nodes appear on the outer electron FS23 to explain their observations. However, there is a discrepancy in the literature on the ARPES data utilizing variable energy photons from synchrotron24,25.

A related system SrFe2(As1−xPx)2 (Sr122P) has a slightly higher optimal critical temperature (x = 0.35, Tc = 33 K) than that of Ba122P (x = 0.30, Tc = 30 K), and its parent compound SrFe2As2 has a much higher Néel temperature (TN = 197 K) than that of BaFe2As2 (TN = 138 K)26. While Sr122P and Ba122P share nearly the same pnictogen heights from the square Fe plane, the c-axis length is significantly shorter in Sr122P than in Ba122P reflecting the smaller ionic radius of the Sr2+ ion than that of the Ba2+ ions. In a previous work on as-grown samples of Sr122P27, we have measured its band dispersions and FSs, and clarified that the outer hole FS is more strongly warped along the kz direction than the corresponding one in Ba122P. The presence of line nodes in Sr122P is also suggested from the 31P-NMR28, specific heat29, and penetration depth measurements30. It is, therefore, conceivable that the same pairing mechanism gives rise to qualitatively similar nodal SC gaps both in Ba122P and Sr122P and also to some differences arising from the accidental nature of line nodes in the s-wave SC state. Thus Sr122P is an ideal system for examining the SC gaps in a systematic way, and new insights into the nodal SC gaps in iron pnictides could be obtained. In particular, the gap function on the more expanded outer hole FS around the Z point may clarify the dominant pairing interaction, because the contribution from the dz2 orbital sensitively controls the magnitude of the SC gaps.

## Results

### Fermi surfaces of SrFe2(As0.65P0.35)2

In-plane FS mapping taken with  = 24 eV and 28 eV is shown in Fig. 1(a,b), respectively. The first BZ of Sr122P is also shown in the inset of (a).  = 24 eV corresponds to a plane slightly above the kz = 2π plane at the zone center, and  = 28 eV crosses the X [(π, π, 2π)] point, judging from the radius of the hole FSs27 and the elongation of the ε FS along the (0, 0, 2π) − (π, π, 2π) line22. There are three hole-like bands crossing EF around the Z point, which form three circular FSs, and two electron-like bands crossing EF around the X point. These FS topologies are the same as those for the as-grown samples27, demonstrating that the annealing process (described in ref.26) does not modify the electronic structure significantly. The dominant orbital character of the hole bands crossing EF are dxz/yz (β, γ) around the Γ point, and dxy (α), dxz/yz (β), and dxz/yz and dz2 (γ) around the Z point. The orbital character for electron bands is dxz/yz (δ) and dxy (ε).

### Superconducting gaps in the hole Fermi surfaces

Now we investigate the SC gap in the momentum space. Figure 2(a) shows FS mapping taken with the 7 eV laser. The observation of three FSs and their radii indicate that  = 7 eV measures a plane close to the Z point. We define the FS angle θ with respect to the nearest-neighbor Fe-Fe direction as indicated in the figure. Symmetrized energy distribution curves (EDCs) below and above Tc for the three FSs are shown in Fig. 2(b–d). The closure of the gap above Tc demonstrates that the gap originates from superconductivity. To extract the gap size from the data, symmetrized EDCs below Tc have been fitted to a phenomenological low-energy spectral function of the form31

$$A({k}_{F},\omega )=-\frac{1}{\pi }\frac{{\Sigma }^{\text{'}\text{'}}({k}_{F},\omega )}{{[\omega -\Sigma ^{\prime} ({k}_{F},\omega )]}^{2}+{[{\Sigma }^{\text{'}\text{'}}({k}_{F},\omega )]}^{2}},$$
(1)

with the self-energy at kF,

$$\Sigma ({k}_{F},\omega )=-\,i{\Gamma }_{1}+{\Delta }^{2}/[\omega +i{\Gamma }_{0}\mathrm{].}$$
(2)

Here, Γ1 is the single-particle scattering rate, Δ is the SC gap, and Γ0 is the inverse pair lifetime. It is known that a finite Γ0 well reproduces the spectral broadening in the pseudogap state of the cuprates31. Although the importance of the Γ0 term has been pointed out23, here we have set Γ0 = 0 because the present symmetrized EDCs do not have maxima at ω = 0 and the EDCs at 40 K (just above Tc = 33 K) in panels (b–d) do not show any signature of pseudogap. When the spectra have clear coherence peaks and deep gaps at ω = 0 as in the α and β FSs, this fitting procedure works well and the gap size thus deduced yields the coherence peak position [panels (b) and (c)]. However, in the absence of clear SC peaks due to the small gap or low quasiparticle weight as in the case of the γ FS [panel (d)], the fitting is quite unstable and a wide range of parameter sets can reproduce the spectral lineshapes, making it difficult to estimate the SC gap values. Therefore, we have estimated the SC gap of the γ FS from the shoulder structures of the low-T spectra if they exist, as indicated by open circles in Fig. 2(d), and we plot only error bars if there is no discernible shoulder structure. We had to resort to visual inspection of the spectra to determine the shoulder positions with larger error bars, but this is partly justified by the fact that the shoulder positions in Fig. 2(d) are in good agreement with the energy at which the changes between the 3 K and 40 K spectra occurs, evidencing that the shoulders are indeed caused by the SC gap opening. We notice that the shoulder positions exhibit an angular dependence, and that the shoulders are almost absent in the −2° and −15° spectra. Note that even when there is no signature of SC gap opening, a positive Δ with comparable Γ1 can reproduce spectra like the −15° one in panel (d), as pointed out by Khodas et al.23. Furthermore, the spectral intensity of the γ band is weaker than that in the other bands. Thus, throughout this paper, we do not claim the presence of nodes simply based on the absence of a gap, as previously done for Ba122P by Zhang et al.24. Instead, our argument is based on the anisotropy of the shoulder structures. The extracted SC gap is plotted in Fig. 2(e) as a function of θ and the dotted lines indicate the fitting of the α/β FS data by Δ(θ) = Δ0 + Δ2 cos(4θ). The α and β FSs have isotropic gaps of Δα(θ) = 5.1 + 0.4 cos(4θ) meV and Δβ(θ) = 4.5 + 0.3 cos(4θ) meV, respectively. On the other hand, the γ FS shows a signature of gap anisotropy with the minimum around θ = 0° and the maxima around θ = 45°.

In order to study a wider momentum range, we employed synchrotron ARPES. Figure 3(a) shows symmetrized energy-momentum (E-k) ARPES intensity plots for the hole FSs taken with  = 23 eV photons, which again corresponds to the kz = 2π plane including the Z point at the zone center. The kF positions are indicated by arrows, and the momentum cuts in the BZ are illustrated in Fig. 3(b). As we have seen in the laser data, the SC coherence peak intensity is the strongest for the α sheet, and the weakest for the γ sheet. The symmetrized EDCs are shown in Fig. 3(c–e). We observe more pronounced SC coherence peaks for the α FS [panel (c)] than the laser data, probably reflecting larger photoemission cross sections at  = 23 eV. For the β FS [panel (d)], the spectral shape is similar to the laser data. For the γ FS [panels (e1) and (e2)], we again observe an indication of anisotropy from the shoulders indicated by the circles. The estimated SC gap is plotted in Fig. 3(f). We again obtain the isotropic gaps of Δα(θ) = 7.5 + 0.1 cos(4θ) meV for the α FS and Δβ(θ) = 6.1 + 0.3 cos(4θ) meV for the β FS. For the γ FS, the amplitude of the anisotropic shoulder is ~5 meV around θ = ±45° and 135°, and a signature of gap minima around θ = 90° (equivalent to θ = 0°), consistent with the laser data. However, we also observe flat symmetrized EDCs between −14° < θ < 49° in Fig. 3(e1,e2), probably because the momentum cuts approach the FS edge, which tends to reduce the photoemission intensity and leads to featureless EDCs.

In order to study the kz dependence of the SC gap, we have performed measurements by varying photon energy. Figure 4(a) shows Ek intensity plots for the hole FSs taken using various photon energies  = 23–31 eV. The momentum cuts are parallel to those in Fig. 3. At the zone center,  = 23 eV corresponds to the Z point and  = 31 eV to the Γ point. We observe a strong warping of the γ FS as is varied, as illustrated in Fig. 4(b). Symmetrized EDCs are plotted in Fig. 4(c–e) and the estimated gap magnitudes are plotted in Fig. 4(f). As kz moves from the Z point toward the Γ point, the gap on the α FS becomes smaller and the coherence peak intensity also becomes lower. The lineshape of the β FS is almost unchanged and the gap is almost constant. For the γ FS, the lineshape is almost unchanged while the gap increases slightly.

### Superconducting gaps in the electron Fermi surfaces

Next we move to the electron FSs. Figure 5(a) shows symmetrized E-k intensity plots for the electron FSs taken with  = 24 eV photons. It can be seen that the SC gap is finite for all the kF’s. Judging from the fact that the two electron FSs are almost circular around the (π,π) point as illustrated in Fig. 5(b),  = 24 eV would correspond to a plane with k ~ π. The symmetrized EDCs are shown in Fig. 5(c,d). We observe SC coherence peaks in the δ sheet. For the ε sheet, although the background level is high due to the presence of the δ band below the ε band, we still observe a gap at ω = 0. The estimated SC gap is plotted in Fig. 5(e). Both the δ and ε FSs have the isotropic SC gaps of Δδ(θ) = 7.0 + 0.2 cos(2θ) + 0.6 cos(4θ) meV and Δε(θ) = 7.8 + 0.0 cos(2θ) + 0.4 cos(4θ) meV. This isotropic gap is in contrast to the observed line nodes22 and gap anisotropy25 in the electron pockets of Ba122P.

To investigate the kz dependence of the gap on the electron FSs, we also performed in-plane measurements with another of 28 eV. Figure 6(a) shows symmetrized E-k intensity plots.  = 28 eV corresponds to the kz = 2π plane including the X point, as illustrated in Fig. 6(b). One again observes that the SC gap is finite for all the kF’s. The symmetrized EDCs are shown in Fig. 6(c,d). The line shapes are close to those in Fig. 5. The SC gap is plotted in Fig. 6(e). Again one obtains almost isotropic gaps of Δδ(θ) = 7.5 + 0.4 cos(2θ) + 0.4 cos(4θ) meV and Δε(θ) = 8.3 + 0.7 cos(2θ) + 0.0 cos(4θ) meV. From these results, one may exclude the possibility of nodes on the electron FSs.

## Discussion

Although it was not possible to determine the three-dimensional nodal structure on the entire FSs from the limited momentum cuts in our measurements, line nodes are most likely located near the crossing point of the θ = 0° line on the γ hole FS around the Z point considering the anisotropic small gap and very weak coherence peaks. Under the condition that the order parameter on the γ FS has the A1g symmetry, a possible scenario of the nodal SC gap structure is the formation of loop-like nodes on the γ hole FS, around the Z point, and around the θ = 0° line (the Z-X line), as illustrated in Fig. 7(b) (details below). We now examine whether an order parameter Δ(k) with A1g symmetry smoothly varying in k space can explain our three-dimensional experimental data and produce loop nodes. To reduce the number of free parameters, we first assume that Δ(k) is kz-independent and that the kz dependence of the SC gap is solely due to the warping of the γ FS along kz. The observed anisotropy of the SC gaps can thus be reasonably reproduced by including four Fourier components: Δ(k) = 1 + 4[cos(kxa) + cos(kya)] − 7 cos(kxa)cos(kya) + 4[cos(2kxa) + cos(2kya)] (meV) [Fig. 7(a)]. On the γ FS, this Δ(k) changes sign around the Z-X line as illustrated in Fig. 7(b), and accordingly produces small loop-like nodes. Figure 7(c,d) show comparison between this Δ(k) and the in-plane experimental data for the γ FS [Fig. 2(e) and 3(f)]. Δ(k) curves at kz = 2π (solid lines) well reproduce the angular dependence of the experimental data. To take into account the possible experimental kz broadening effect in the low-energy ARPES, Δ(k) curves at kz = 2.4π are also shown as dotted lines. The kz broadening further improves the fit, since Δ(k) becomes always positive when kz moves away from 2π. As shown in Fig. 7(e), the gradual increase of the gap along the kz direction [Fig. 4(f)] is also well captured in the fitting. The present analysis demonstrates that the above kz-independent order parameter can reasonably describe the observed SC gap in a large portion of the three-dimensional γ hole FS, obviating the need for introducing three-dimensional Fourier components and their fine-tuning. However, as theoretical studies have indicated, Δ(k) may have intrinsic kz dependence, particularly when the dominant orbital component changes along kz. In Sr122P, the dz orbital contribution is strongly suppressed as kz goes away from the Z point, which necessitates the inclusion of kz2 dependence in Δ(k). Indeed, this would further improve the agreement with the experimental data in Fig. 7. In particular, the size of the negative SC gap region can be fine-tuned and the kz dependence in Fig. 7(e) would be better fitted with the three-dimensional Δ(k). The overall topology of SC gap structure, however, remains the same as Fig. 7(b) if the three-dimensionality is weak. On the other hand, strong three-dimensionality of Δ(k) may generate other possible nodal SC gap structures, such as the three-dimensional, anisotropic SC gap on the entire γ FS. In this case, closely spaced two vertical line nodes (hence eight vertical line nodes in total) would be formed on the γ FS.

Here we discuss the comparison of the present result with the theoretical calculations on Ba122P in the literature. Suzuki et al.18 calculated the gap structure of Ba122P based on the spin-fluctuation exchange mechanism and showed that sign reversal occurs on the γ FS around the Z point, consistent with the present result. Quantitatively speaking, however, their result shows that the sign-reversed gap on the γ FS has a (negative) maximum along the direction 45° off the Z-X direction, which is rotated from the present result. On the other hand, Saito et al.19 showed that the SC gap on all the hole FS becomes of the same sign, the gap on the electron FSs becomes anisotropic, and nodes may be formed on the electron FSs depending on the magnitude of microscopic parameters. Also, the gap of the hole FSs on the kz = π plane is the largest for the γ FS. Since the γ FS in Sr122P is more strongly warped than Ba122P due to the smaller c-axis lattice parameter, the theoretical SC gap structure on the γ FS of Sr122P could be largely modified from those of Ba122P. A direct calculation of Sr122P using its lattice parameters would further facilitate the understanding of microscopic pairing mechanism both in Ba122P and Sr122P.

Finally, we would like to make a remark on the effect of impurities on the SC gap structure. A recent study on the effects of electron irradiation and natural disorder in Sr122P single crystals32 showed that the low-temperature behavior of the penetration depth can be described by a power-law function Δλ(T) = ATn, with n close to one for pristine annealed samples and larger than two for electron-irradiated ones, implying that the nodes are accidental and can be lifted by the introduction of disorder. For Ba122P, Mizukami et al.16 also found that the nodal state changes to a nodeless state showing fully gapped excitations by introducing nonmagnetic point defects by electron irradiation. Theoretically, Kontani et al.7 proposed a possibility of crossover from s± wave to s++ wave with increasing the impurity concentrations. The present annealed samples, which yielded n ~ 1 in Strehlow et al’s penetration depth measurement32, can be reasonably regarded as “pure”, and a comparison with theory with low impurity concentration is justified. To further clarify this issue, direct ARPES investigation into the change of SC gap structure with different impurity concentrations is left for future studies.

In conclusion, we have measured the SC gaps of optimally-doped Sr122P in wide three-dimensional momentum space by laser-based and synchrotron-radiation ARPES. Around the Z point, the α and β hole FSs have isotropic SC gap of 8 meV and 6 meV, respectively. The gap on the γ FS is anisotropic with the amplitude of 5 meV with minima located along the Z-X direction. The electron FSs have isotropic gap of 8 meV, which is almost independent of the kz. As for the possible location of line nodes, we propose that there exists a sign change on the γ hole FS, around the Z point, and around the Z-X line. A direct theoretical calculation of the Sr122P SC gap structure using its lattice parameters, together with the existing data on Ba122P and Sr122P, would further deepen our understanding of the nodal superconductivity in the iron pnictides.

## Methods

Sr122P single crystals were prepared by the self-flux method described in ref.29 and postannealed to achieve the optimal Tc of 33 K26. The Tc was determined by the onset of Meissner diamagnetic signal with the transition width of ΔTc 5 K. ARPES experiments were carried out at beamline 5–4 of Stanford Synchrotron Radiation Lightsource (SSRL) and at a laser ARPES apparatus at Institute for Solid State Physics (ISSP). In order to obtain clean surfaces, samples were cleaved in situ at pressure better than 1 × 10−10 Torr. Cleavage occurs along the ab planes. The kinetic energies and momenta of photoelectrons were measured using Scienta R4000 electron energy analyzers. In the following, the x and y axes point from Fe towards the nearest neighbor Fe atoms, the X and Y axes point from the Fe atom towards the second nearest-neighbor Fe atoms, and the z axis is parallel to the c-axis. In-plane (kX, kY) and out-of-plane momenta (kz) are expressed in units of 1/a and 1/c, respectively, where a = 3.90 Å and c = 12.09 Å are the in-plane and out-of-plane lattice constants. Calibration of the Fermi level (EF) was achieved using the spectra of gold which was in electrical contact with the samples. Incident photons from 21 eV to 35 eV from the synchrotron were linearly p-polarized. For laser ARPES, the incident photons with  = 6.998 eV were linearly s-polarized. The total energy resolution was ΔE ~ 6 meV at T = 5 K for synchrotron-radiation ARPES, and ΔE ~ 1 meV at T = 3 K for laser ARPES.

## Data availability

The data sets generated during and/or analysed during the current study are available from the corresponding author on reasonable request.

## References

1. 1.

Kamihara, Y., Watanabe, T., Hirano, M. & Hosono, H. Iron-based layered superconductor La[O1−xFx]FeAs (x = 0.05–0.12) with T c = 26 K. J. Am. Chem. Soc. 130, 3296–3297 (2008).

2. 2.

Hirschfeld, P. J., Korshunov, M. M. & Mazin, I. I. Gap symmetry and structure of Fe-based superconductors. Rep. Prog. Phys. 74, 124508 (2011).

3. 3.

Chubukov, A. Pairing mechanism in Fe-based superconductors. Annu. Rev. Cond. Matter Phys 3, 57–92 (2012).

4. 4.

Kuroki, K. et al. Unconventional pairing originating from the disconnected Fermi surfaces of superconducting LaFeAsO1−xFx. Phys. Rev. Lett. 101, 087004 (2008).

5. 5.

Mazin, I. I., Singh, D. J., Johannes, M. D. & Du, M. H. Unconventional superconductivity with a sign reversal in the order parameter of LaFeAsO1−xFx. Phys. Rev. Lett. 101, 057003 (2008).

6. 6.

Scalapino, D. J. A common thread: The pairing interaction for unconventional superconductors. Rev. Mod. Phys. 84, 1383–1417 (2012).

7. 7.

Kontani, H. & Onari, S. Orbital-fluctuation-mediated superconductivity in iron pnictides: Analysis of the five-orbital Hubbard-Holstein model. Phys. Rev. Lett. 104, 157001 (2010).

8. 8.

Onari, S. & Kontani, H. Self-consistent vertex correction analysis for iron-based superconductors: Mechanism of Coulomb interaction-driven orbital fluctuations. Phys. Rev. Lett. 109, 137001 (2012).

9. 9.

Thomale, R., Platt, C., Hanke, W., Hu, J. & Bernevig, B. A. Exotic d-wave superconducting state of strongly hole-doped KxBa1−xFe2As2. Phys. Rev. Lett. 107, 117001 (2011).

10. 10.

Maiti, S. & Chubukov, A. V. s+is state with broken time-reversal symmetry in Fe-based superconductors. Phys. Rev. B 87, 144511 (2013).

11. 11.

Lin, S.-Z., Maiti, S. & Chubukov, A. Distinguishing between s+id and s+is pairing symmetries in multiband superconductors through spontaneous magnetization pattern induced by a defect. Phys. Rev. B 94, 064519 (2016).

12. 12.

Scalapino, D. The case for d x 2 y 2 pairing in the cuprate superconductors. Phys. Rep 250, 329–365 (1995).

13. 13.

Kasahara, S. et al. Evolution from non-Fermi- to Fermi-liquid transport via isovalent doping in superconductors. Phys. Rev. B 81, 184519 (2010).

14. 14.

Nakai, Y. et al. 31P and 75As NMR evidence for a residual density of states at zero energy in superconducting BaFe2 (As0.67P0.33)2. Phys. Rev. B 81, 020503 (2010).

15. 15.

Hashimoto, K. et al. Line nodes in the energy gap of superconducting BaFe2(As1−xPx)2 single crystals as seen via penetration depth and thermal conductivity. Phys. Rev. B 81, 220501 (2010).

16. 16.

Mizukami, Y. et al. Disorder-induced topological change of the superconducting gap structure in iron pnictides. Nat. Commun. 5, 5657 (2014).

17. 17.

Kuroki, K., Usui, H., Onari, S., Arita, R. & Aoki, H. Pnictogen height as a possible switch between high- T c nodeless and low-T c nodal pairings in the ironbased superconductors. Phys. Rev. B 79, 224511 (2009).

18. 18.

Suzuki, K., Usui, H. & Kuroki, K. Possible three-dimensional nodes in the s± superconducting gap of BaFe2(As1−xPx)2. J. Phys. Soc. Jpn. 80, 013710 (2011).

19. 19.

Saito, T., Onari, S. & Kontani, H. Nodal gap structure in Fe-based superconductors due to the competition between orbital and spin fluctuations. Phys. Rev. B 88, 045115 (2013).

20. 20.

Shimojima, T. et al. Orbital-independent superconducting gaps in iron pnictides. Science 332, 564–567 (2011).

21. 21.

Shimojima, T. et al. Angle-resolved photoemission study on the superconducting iron-pnictides of BaFe2(As1−xPx)2 with low energy photons. Solid State Commun 152, 695–700 (2012).

22. 22.

Yamashita, M. et al. Nodal gap structure of superconducting BaFe2(As1−xPx)2 from angle-resolved thermal conductivity in a magnetic field. Phys. Rev. B 84, 060507 (2011).

23. 23.

Khodas, M. & Chubukov, A. V. Vertical loop nodes in iron-based superconductors. Phys. Rev. B 86, 144519 (2012).

24. 24.

Zhang, Y. et al. Nodal superconducting-gap structure in ferropnictide superconductor BaFe2(As0.7P0.3)2. Nat. Phys 8, 371–375 (2012).

25. 25.

Yoshida, T. et al. Anisotropy of the superconducting gap in the iron-based superconductor BaFe2(As1−xPx)2. Sci. Rep 4, 7292 (2014).

26. 26.

Kobayashi, T., Miyasaka, S., Tajima, S. & Chikumoto, N. Electronic phase diagram of SrFe2(As1−xPx)2 : Effect of structural dimensionality. J. Phys. Soc. Jpn. 83, 104702 (2014).

27. 27.

Suzuki, H. et al. Strongly three-dimensional electronic structure and Fermi surfaces of SrFe2(As0.65P0.35)2 : Comparison with BaFe2(As1−xPx)2. Phys. Rev. B 89, 184513 (2014).

28. 28.

Dulguun, T. et al. Unconventional multiband superconductivity with nodes in single-crystalline SrFe2(As0.65P0.35)2 as seen via 31P NMR and specific heat. Phys. Rev. B 85, 144515 (2012).

29. 29.

Kobayashi, T. et al. Change of electronic state and crystal structure by postannealing in superconducting SrFe2(As0.65P0.35)2. Phys. Rev. B 87, 174520 (2013).

30. 30.

Murphy, J. et al. Nodal superconductivity in isovalently substituted SrFe2(As1−xPx)2 pnictide superconductor at the optimal doping x = 0.35. Phys. Rev. B 87, 140505 (2013).

31. 31.

Norman, M. R., Randeria, M., Ding, H. & Campuzano, J. C. Phenomenology of the low-energy spectral function in high- Tc superconductors. Phys. Rev. B 57, 11093–11096 (1998).

32. 32.

Strehlow, C. P. et al. Comparative study of the effects of electron irradiation and natural disorder in single crystals of SrFe2(As1−xPx)2 superconductor (x = 0.35). Phys. Rev. B 90, 020508 (2014).

## Acknowledgements

We are grateful to M. Nakajima and H. Eisaki for enlightening discussions. Stanford Synchrotron Radiation Lightsource is operated by the Office of Basic Energy Science, US Department of Energy. H.S. and M. Horio acknowledge financial support from Advanced Leading Graduate Course for Photon Science (ALPS) and the JSPS Research Fellowship for Young Scientists. This work was supported by JSPS KAKENHI Grant NumbersJP19K03741, JP19H00651, JP19H01818, JP19H05826.

## Author information

Authors

### Contributions

H.S. and K.O. performed Laser ARPES experiment with the help of Y.O., H.Y. and S.S. H.S., K.O., T.Y., M. Horio and L.C.C.A. performed synchrotron ARPES experiment with the help of M. Hashimoto., D.H.L. and Z.X.S. T.K., S.M. and S.T. grew the Sr122P single crystals and performed sample characterizations. H.S. analyzed the experimental data. H.S. and A.F. wrote the manuscript with comments from all co-authors.

### Corresponding authors

Correspondence to H. Suzuki or A. Fujimori.

## Ethics declarations

### Competing interests

The authors declare no competing interests.

Publisher’s note Springer Nature remains neutral with regard to jurisdictional claims in published maps and institutional affiliations.

## Rights and permissions

Reprints and Permissions

Suzuki, H., Kobayashi, T., Miyasaka, S. et al. Band-dependent superconducting gap in SrFe2(As0.65P0.35)2 studied by angle-resolved photoemission spectroscopy. Sci Rep 9, 16418 (2019). https://doi.org/10.1038/s41598-019-52887-y

• Accepted:

• Published: