To probe the remarkable nature of defect excitations in the superconducting TSS, we deposit magnetic Fe adatoms on the cleaved (001) surface of a single crystal of FeTe0.55Se0.45 (Fig. 1a-b) with the substrate temperature below 20 K. Before depositing the Fe adatoms, we scan the surface to ensure that there is no interstitial Fe adatom (See Supplementary Note I), to avoid the mix of interstitial Fe adatoms and deposited Fe adatoms. In contrast to the growth-induced interstitial Fe impurity in the bulk, the adsorbed Fe adatoms are distributed at varies heights above the surface and in different planar locations with respect to the C4 symmetry sites. As a result, the magnetic Fe adatoms with varying exchange couplings reveal much richer phenomena of the defect excitations of the superconducting TSS.
The STM image of a surface region after the atomic deposition (Fig. 1c) shows scattered Fe adatoms as the bright spots with a coverage of ~0.04 %. The zero-energy dI/dV map in the same area of Fig. 1c, displays relatively high density of states at the locations of the Fe adatoms (Fig. 1d), consistent with the physical picture that magnetic Fe impurities generate in-gap states. From the statistics of more than one hundred measurements (Supplementary Note I, Fig. S2), we identify two types of in-gap states localized around the Fe adatoms with distinct dI/dV spectra exemplified in Fig. 1e. The type-I adatoms, which represent about 10% of our measurements, exhibit a sharp ZBP reminiscent of a MZM coexisting with other in-gap states in the dI/dV spectrum. In contrast, the conductance spectrum of the type-II adatoms, which represent about 90% of our measurements, shows the YSR states, featuring a pair of in-gap states at particle-hole symmetric peak energy positions, but with asymmetric peak weights. In comparison, the typical dI/dV spectrum on the clean surface without the adatom shows a hard superconducting gap without in-gap states (Fig. 1e).
We begin with the type-I Fe adatoms. A high-resolution topographic image (Fig. 2a) shows an isolated type-I adatom. A circular pattern appears in the zero-energy dI/dV map in the vicinity of the Fe site (Fig. 2b), with the zero-energy intensity center slightly offset from the Fe site. The waterfall-like dI/dV spectra (Fig. 2c) and the intensity plot (Fig. 2d) along the red dashed line-cut in Fig. 2a clearly resolve the ZBP and other peaks at nonzero energies inside the superconducting gap. The ZBP persists to about 2.5 nm from the center, indicating the existence of a localized zero-energy state bound to the Fe adatom with the spatial extent comparable to that of the MZM in a magnetic field-induced vortex core in FeTe0.55Se0.456. To explore the nature of the discretized in-gap states, we extract several dI/dV spectra from Fig. 2c and show them as a stacking plot in Fig. 2e. Doing so accounts for the spatial distributions of the in-gap states and the sample inhomogeneity6, 7 due to Te/Se alloying, which has proven to be useful for studying the core states of magnetic field-induced vortices in FeTe0.55Se0.458. The sequence of discretized bound states, including the zero-energy state, is clearly visible as the pronounced peaks labeled by L0, L±1, L±2. The energy positions of the conductance peaks (Ln) are plotted in Fig. 2f. Intriguingly, the average energies (solid lines) of the discrete quantum states bound to the Fe adatom follow closely a sequence of integer quantization , with the minigap meV, the same integer sequence (with a minigap ~ 0.6 meV) followed by the quantized vortex core states observed recently8 in magnetic field-induced vortices that host the MZM6, 7. The different values of the minigap are caused by the fluctuation of the superconducting gap Δ and Fermi energy Ef on different surface, due to the inhomogeneous Te and Se atoms in FeTe0.55Se0.45. More cases are shown in Supplementary Fig. S3 for the type-I Fe adatoms. Such an integer quantized sequence is the hallmark of the CdGM vortex core states of the superconducting TSS in the quantum limit8, 28. Our observations thus provide substantiated and compelling evidence that vortex-like topological defect excitations such as the QAVs nucleate spontaneously at the type-I Fe adatoms and the ZBP corresponds to a vortex MZM.
It is necessary to check the temperature and magnetic field dependence of the ZBP, since a vortex MZM would respond differently than vortex-free defect states. The temperature evolution of the ZBP on the Fe adatom turns out to be very similar to that of the MZM in a field-induced vortex6. The ZBP intensity of the center spectrum pointed by the black arrow in Fig. 2c decreases with increasing temperatures, and becomes almost invisible at 4.2 K (Fig. 2g). The magnetic field dependence is also very similar to that of a vortex MZM as the ZBP does not split or broaden for fields up to 8 T (Fig. 2h), provided that no field-induced vortices enter the region near the adatom when the magnetic field is applied. The ZBP is however sensitive to the location of the adsorbed Fe adatom. We found that all type-I adatoms producing integer quantized bound states anchored by the ZBP are adsorbed at the high-symmetry sites in the center of four Te/Se atoms. To test the robustness of this finding, we manipulate a type-I adatom by the STM tip to a different location away from the C4 symmetric site. The ZBP disappears and a pair of in-gap state at nonzero energy emerges (Supplementary Note III and Fig. S4). After annealing the sample to 15 K and perform the measurement again at 0.4 K, the adatom diffuses back to its original high-symmetry site and the ZBP reappears. Thus, the high-symmetry site is a prerequisite for the induced ZBP, which agrees with the proposed theory that the orbital magnetic moment of the Fe adatoms at C4 symmetric locations plays an important role for the nucleation of the QAV28.
Next, we turn to study the type-II Fe adatoms (Supplementary Note IV). In contrast to the type-I adatoms, the conductance exhibits predominantly a pair of in-gap peaks at nonzero energies without the ZBP. Applying an external magnetic field, we observe that the peaks shift approximately linearly to higher energies (Supplementary Fig. S5d) away from the Fermi level, consistent with a pair of spin-polarized YSR in-gap states. We find that the type-II Fe adatoms are adsorbed at myriad locations on or off the high-symmetry axis and induce YSR states at different energies, indicative of broadly varying exchange couplings to the superconducting quasiparticles. In special cases, we also observe YSR states located very close to zero energy, which nevertheless split under the magnetic field (Supplementary Note IV and Fig. S6) and are therefore distinct from the robust ZBP observed on the type-I Fe adatoms.
These observations motivate us to manipulate the exchange coupling between the magnetic adatoms and the substrate by tuning the tip to sample distance29, 30. The electrostatic force of an approaching tip can prod and move the Fe adatom in directions parallel and perpendicular to the surface (Fig. 3a), which can affect the atomic orbital moment of the Fe adatom and the spin-orbit exchange coupling to the superconductor. In STM/S, the tunnel-barrier conductance GN , where It is the tunneling current and Vs is the bias voltage, governs the tunnel coupling and changes with the tip-sample distance. Performing tunneling conductance measurements as a function of GN, we find that the energies of the YSR states are modulated ubiquitously when the tip approaches the type-II Fe adatoms (Supplementary Note V). The observed crossing and reversal of the in-gap states (Supplementary Fig. S7), a trademark of the YSR states, confirms that reducing the tip to sample distance monotonically increases the exchange coupling between the Fe atom and the superconductor.
Unexpectedly, as the STM tip approaches a significant number of the type-II Fe adatoms (~ 27%), the pair of YSR states modulates with increasing GN, but then coalesces in a captivating manner into a single ZBP in the water-fall plot of dI/dV spectra (Fig. 3c) and the intensity plot (Fig. 3d), which remains robust under further increase of the barrier conductance. Note that the emergence of the ZBP out of the YSR states is different from the transition point between the screened spin-singlet and doublet ground states29, 31, where the two YSR states are approximately degenerate at zero energy as marked by the red arrow in Fig. 3d. To probe the change in the nature of the in-gap states with different barrier conductance, we repeated the entire process under an applied magnetic field. The dI/dV spectra and the intensity plot obtained under 6 T (Fig. 3e-f) show that the vortex-free YSR states no longer cross zero energy, due to the Zeeman splitting that removes the accidental degeneracy. However, the emergence of the unsplit ZBP at higher GN is unabridged even at such a high field, indicating that ZBP corresponds to a single MZM robust against an applied magnetic field. This identification is further corroborated by performing the measurements on type-I Fe adatoms that show the ZBP associated with the MZM upholds its integrity and does not shift or split with increasing GN in a field as high as 6 T (Supplementary Note VI and Fig. S8). The compelling evidence attributes the novel coalescence of in-gaps states to the ZBP as a topological transition (Fig. 3b) from the vortex-free YSR states to a vortex MZM, which is fully consistent with the theoretical prediction that increasing the exchange coupling of an Fe impurity induces a transition from the YSR states to the QAV states hosting a MZM in FeTe0.55Se0.45 superconductors28. The transition between the YSR states and the MZM is even reversible, as the dI/dV spectra as a function of the barrier conductance retrace that shown in Fig. 3e-f upon withdrawing the tip (Fig. 3g-h) in a controlled manner. The transition is also replicable when the type-II Fe adatom under the tip in Fig. 3 is moved to a different location about 1 nm away (Supplementary Fig. S9). These observations reveal the unprecedented nature of defect excitations in the superconducting TSS where local magnetic moment and screening currents are inextricably connected through the magnetoelectric effect.
The phase coherence of the MZMs is stored nonlocally and protected by the topological degeneracy against the ravages of environmental decoherence caused by local perturbations, which is the central to the idea of topological quantum computing32, 33. The coupling of two MZMs sufficiently close by annihilates of the nonabelian anyonic zero modes and creates a pair of fermionic states at nonzero energies. This fusion process usually requires two overlapping magnetic field induced vortices, which is difficult to control on the Abrikosov lattice7, 8, 34. Our system allows a new possibility, i.e., the fusion between MZMs hosted in a QAV and a field-induced vortex (Fig. 4). The zero-energy dI/dV map (Fig. 4a) shows a MZM in the QAV nucleated at a type-I Fe adatom in a magnetic field of -0.2 T, also visible in the intensity plot (Fig. 4b) as sharp ZBPs along the line cut across the adatom. A field-induced vortex is observed to enter the field of view subsequently. The latter sits very close to the Fe site, thus enlarges significantly the region with spectral weight at zero-energy (Fig. 4c). Remarkably, acquiring the intensity plot along the same line cut shows that the ZBP splits into two peaks separated by an energy spacing ~ 0.25 meV (Fig. 4d). During the second round of the measurements, the vortex creeps away. The zero-energy map recovers (Fig. 4e) and the ZBP reemerges in the intensity plot (Fig. 4f). Throughout the fusion process, the temperature and the magnetic field are kept stable. It is necessary to point out that the creeping of the vortices is observed quite often when we detected MZMs in the filed-induced vortices in our previous work. Three representative dI/dV spectra corresponding to the three conditions are extracted and displayed in Fig. 4g for a better comparison. Repeating the measurements on the same Fe adatom in a higher magnetic field of -3 T reveals again the splitting of the ZBP caused by the presence of a nearby field-induced vortex (Fig. 4h), with a larger energy spacing ~ 0.35 meV (Fig. 4i), possible due to the shorter distance and stronger overlap of the two MZMs as indicated by the smaller ring feature in the zero-energy map in Fig. 4h compared to Fig. 4c. Moreover, a field-induced vortex can also enter the field of view without causing detectable splitting of the ZBP bound to the Fe adatom or the vortex MZM when they are relatively far apart (Supplementary Note VIII and Fig. S10). These observations further support the identification of the ZBP induced by type-I Fe atoms as the MZM and concurrently provide the first experimental evidence for the fusion between two vortex MZMs as illustrated in Fig. 4j.