Magnetic skyrmions are topologically stable whirlpool-like spin textures that offer great promise as information carriers for future spintronic devices. To enable such applications, particular attention has been focused on the properties of skyrmions in highly confined geometries such as one-dimensional nanowires. Hitherto, it is still experimentally unclear what happens when the width of the nanowire is comparable to that of a single skyrmion. Here, we achieve this by measuring the magnetoresistance in ultra-narrow MnSi nanowires. We observe quantized jumps in magnetoresistance versus magnetic field curves. By tracking the size dependence of the jump number, we infer that skyrmions are assembled into cluster states with a tunable number of skyrmions, in agreement with the Monte Carlo simulations. Our results enable an electric reading of the number of skyrmions in the cluster states, thus laying a solid foundation to realize skyrmion-based memory devices.
The emergence of topological phenomena and topological materials has attracted growing interests in condensed matter physics1. The interplay between topology and geometry not only deepens our physical understanding, but also provides new routes to device designs that incorporate novel physics. In magnetic materials, a notable example of a topologically stable object is the skyrmion, a swirl-like spin texture that carries quantized topological charge2,3,4,5,6,7,8,9. Skyrmions have been realized in several helimagnets with the non-centrosymmetric B20 crystal structure, such as MnSi, FeGe and FexCo1−xSi2,5,6. The peculiar twists of the magnetization within the skyrmion originate from the competition between the chiral Dzyaloshinskii–Moriya (DM) interaction and the ferromagnetic (FM) exchange interaction. The ratio of these two interactions determines the skyrmion size, which is typically on the order of 5–100 nm, and can be continuously tuned by doping10. Moreover, recent experiments found that skyrmions can be manipulated by electric currents with a current density several orders of magnitude lower than that needed to drive ferromagnetic domain walls4,11. Although these properties are advantageous for high-density data storage applications with low dissipation, most skyrmions in bulk samples or two-dimensional films reported in literatures have condensed into lattices6, which makes the single bit operation impossible. Experimental investigations of epitaxial MnSi/Si(111) films in strong in-plane magnetic field have discovered distorted skyrmion strings12, wherein the strain-induced magnetic anisotropy by the Si substrate is crucial for the stabilization of spin textures, and skyrmions are still aligned in one dimension. Although recent study enables an electric reading of the number of turns in the helical structure in MnSi thin films13, there is a lack in the detection of creation and annihilation of individual skyrmions in devices by an electric probe that can be more readily integrated into conventional electronic architectures14.
Single-crystal nanowires (NWs) of the compounds with the B20 structure provide a valuable insight into this issue15. Skyrmion states have been identified in B20 MnSi NWs by Lorentz transmission electron microscopy16 and longitudinal magnetoresistance (MR) measurements17. However, the widths of the NWs (d>200 nm) in these studies are much larger than the skyrmion lattice constant (Ld∼18 nm) for MnSi, implying that the skyrmion state therein still condenses into the lattice as in bulk samples. Fortunately, our recent advances in nanomaterials allow us to synthesize high-quality crystalline MnSi NWs of various diameters down to tens of nanometres comparable to the skyrmion size, and conveniently manipulate the thin NWs (see Supplementary Fig. 1 for detailed descriptions of the technology). It is thus an interesting question whether skyrmions can survive in such narrow NWs and behave distinctly.
In this work, we demonstrate the formation of individual skyrmions in thin MnSi NWs monitored by MR measurements. A skyrmion cluster18,19, composed of sparsely distributed skyrmions rather than skyrmion lattices, is demonstrated in this confined system under an external magnetic field, B, aligned along the axis of the wire and confirmed by Monte Carlo (MC) simulations. The MR(B) curves exhibit striking jumps at specific fields that corresponds to the creation or annihilation of individual skyrmions. Moreover, the number of jumps depends on the NW diameter, and eventually disappears both in wider and ultra-narrow NWs. Therefore, the jumps in the MR curves reveal the physical signature of the cascading transition of the skyrmion cluster states, and enable an electric reading of the single skrymion.
Magnetotransport properties of 40 nm NW
MnSi NWs were synthesized by chemical vapour deposition15. A representative scanning electron microscopy image of a single wire with a smooth (111) surface is shown in Fig. 1a. The cross-section of the NW shows a merohedral twinning structure with the (001) twin plane parallel with the <110> growth direction (Fig. 1b). This is a common feature of NWs of non-centrosymmetric B20 compounds, in which the unique (001) twin plane partitions the NW into two parts with opposite handedness20. A high-resolution transmission electron microscopy (TEM) image (Fig. 1c), together with previous TEM diffraction results15, confirms the perfect B20 crystal structure. MR measurements were carried out by a standard four-probe technique on individual NWs (the device is illustrated in Supplementary Fig. 2). We selected a 40 nm diameter NW, the size of which is comparable to Ld∼18 nm, to demonstrate the central results. Both resistance (R) versus temperature (T) and MR–T curves are shown in Fig. 1d, where MR at field, B, is defined as MR=[R(B)−R(0 Oe)]/R(0 Oe). The residual resistivity ratio of the wire is R(300 K)/R(5 K)∼7.5. The Curie temperature Tc of the NW is determined to be ∼29 K from Fig. 1d, which is almost the same as that of bulk MnSi (29.5 K). The room temperature resistivity, ρ≈198 μΩ cm, is quite close to the value of 180 μΩ cm reported for bulk single-crystal MnSi21. These results reflect the high quality of the NWs.
Figure 2 shows a typical curve of MR as a function of B for the 40 nm NW at T=14 K. The origin of the MR is ascribed to the coupling of conduction electrons with chiral modulations22,23. Previous theoretical calculation24 and experimental works on MnSi samples17,25,26 have well established that the magnetic scattering of the conduction electrons by the skyrmion phase would lead to two kinks in the MR(B) isotherms, which correspond to the lower and upper critical fields driving the system into and out the skyrmion phase. The data were recorded by increasing the field from −8 kOe to 8 kOe. Following this field-sweeping sequence, and in the MR(B) curve define the transition fields from helical to the skyrmion, and the skyrmion to ferromagnetic phase, respectively24,25,26, or vice versa, where the superscript ‘+ (−)’ denotes the positive (negative) branch of the sweeping field. In contrast to the continuous MR(B) curves for thick wires (>200 nm; ref. 17), this MR(B) curve displays two discontinuous jumps with almost the same amplitudes in the skyrmion phase of BS<B<BF. This difference comes from the fact that the skyrmion lattice cannot be supported in the cross-section of such a narrow NW. Instead, a skyrmion cluster state (SC) with sparsely distributed skyrmions is present18,19. As the skyrmion is a topologically stable spin texture with an apparent particle character, a single skyrmion in the SC cannot be created or destroyed by smooth variation of local moments from other phases. Thus, a field-driven cascading quantized transition is a natural result when the number of skyrmions, Ns, changes one by one under B. The maximum number, Nmax, in a skyrmion cluster state can be easily estimated18,19. As discussed above, the presence of a merohedral twin boundary splits the parallelogram cross-section into two triangles20. Simple geometry analysis suggests that one skyrmion at most can exist in each triangle, resulting in a total number of Nmax=2. This number perfectly matches the number of discontinuous jumps (or drops) in MR.
Simulated spin textures in 40 nm NW
This interpretation of the MR results is further supported by MC simulations based on the actual sample geometry, in which the 40 nm NW is divided into two merohedral lattices. Details of the model are described in the numerical Methods section. Snapshots of both three-dimensional (3D) and the cross-sectional spin configurations are shown in Fig. 3a–f, where the magnetic field B has the unit BR=J/μB, with J the exchange constant and μB the Bohr magneton. At a low field, a distorted helical order is established with the propagation direction lying in the cross-section and perpendicular to the twin boundary (Fig. 3a). This is different from the conventional bulk sample, where the propagation is along the <111> direction due to weak crystal anisotropy2. This difference comes from the presence of the twin boundary, at which the DM interaction vanishes and only ferromagnetic exchange interaction survives. Therefore ferromagnetic ordering is persistent along the twin boundary plane, and modulation along the NW is prohibited. When the field B/BR is increased above a threshold, the skyrmion cluster appears (Fig. 3c). Due to the geometric confinement, only one skyrmion is allowed in each merohedral domain and the skyrmions are aligned along the NW, forming two skyrmion tubes. At the NW boundary, spins align parallel to the boundary due to the DM interaction and missing spins near the boundary18,19,27. Consequently, the swirling direction at the boundary of each domain is opposite to that of the skyrmion within, and each skyrmion tries to sit at the centre of each domain owing to the repulsion from the edge states7,8. Notice that before entering skyrmion cluster state, the system undergoes an intermediated state (Fig. 3b), characterized by forming half-skyrmions in the interior of the NW. As a result, this state weakens the abrupt transition from the helical state into the skyrmion phase, being consistent with the unapparent transition field BS in Fig. 2. With further increase of the field strength, one skyrmion disappears, leaving a mixed state of the 3D modulation in one domain and a skyrmion tube in the other domain (Fig. 3d). Although in the simulations, the geometries of the two domains in the NW are identical except for different chiralities, the ferromagnetic exchange at the twin boundary gives rise to certain correlations between two domains. Our result shows that the formation of 3D modulations in one domain can stabilize the remaining skyrmion in the other, so that two skyrmions do not disappear simultaneously. In real samples, the sizes of the two twins are not exactly identical, which may also lead to the difference in the corresponding critical fields. At an even larger field, the remaining skyrmion transforms into the fully polarized ferromagnetic state (Fig. 3f) via distorted conical (C) phase in a tiny magnetic field interval (Fig. 3e), while swirling along the boundary persists (Fig. 3f). The phase diagram for these states is shown in Fig. 3g. This two-step destruction of the SC state corresponds to the two jumps observed in the MR(B) curve.
The size dependence of magnetotransport properties
The resistance jumps are persistent at various temperatures, as shown in Fig. 4a. However, they gradually evolve into kinks at higher temperatures, because thermal fluctuations smear out the topological transitions. Although the kinks become indistinct above 19 K, a closer examination of the dMR/dB data (Fig. 4b) still shows two peaks between BS and BF, indicating the survival of the two-skyrmion cluster. Symmetric behaviours are shown in both positive and negative branches of the sweeping fields at high temperatures. However, when the temperature drops <15 K, the magnetization kinetics plays an increasingly important role, as indicated by the reappearance of the conical phase, shown by kinks instead of jumps observed at BF in the negative field branches17. This conical phase survives in a narrow window sandwiched between BF and BC shown in Fig. 4a.
Figure 4c shows the T–B phase diagram constructed from transport measurements, in which the solid symbols are derived from BS, BC and BF in the MR(B) curves and the open symbols come from the transition temperature TS1 and TS2 in the MR(T) curves at fixed B (Supplementary Fig. 3). It is found that skyrmion clusters with different Ns are stabilized widely in the T–B plane, ranging from the Tc down to 5 K on the positive field branch, while eclipsed by the conical state in a narrow window at low temperatures on the negative branch. The saturation field BF is lower than that previously reported (6 kOe at low temperatures) for bulk MnSi crystals21 and thick MnSi wires17.
To further understand the importance of NWs size and geometric confinement, we systematically investigated the transport properties of NWs with different diameters (Supplementary Fig. 4). Figure 5a–c show typical MR curves for three NWs with diameters of 80, 55 and 20 nm at representative temperatures. The corresponding dMR(B)/dB data are simultaneously plotted as grey dotted lines to identify the phase transitions clearly. More discontinuous jumps are observed at a thicker NW with a diameter of 55 nm. A detailed analysis clearly shows three additional jumps with similar jump height in the interval BS<B<BF, as labelled in Fig. 5b. A similar numerical calculation shows that only two skyrmions can exist in each triangle divided by the twin boundary, and therefore Nmax=4, which perfectly matches the number of jumps (Supplementary Fig. 5). Comparing Fig. 5b and Fig. 4a, we see that the thinner the NW is, the more prominent the discontinuous jumps are. This can be understood phenomenologically from the anisotropic MR28, which obeys ρ(θ)=ρ0–ρA cos2θ, where θ is the angle between local moments and the cross-section, and the residual resistance ρ0 is much larger than the anisotropic MR ρA. The presence of a skyrmion leads to the spatial modulation of local moments, average over which gives the MR of the wire. It can be easily shown that the resistance change on placement a single skyrmion is given by , where R is the skyrmion radius and c is a dimensionless quantity of unity order. Therefore the larger the sample size is, the smaller the jump height will be, as shown in Fig. 5b. We also notice that the jumps in the negative branches are more obvious than those in the positive ones, reinforcing the important role that the magnetization kinetics plays. The observed exceptional data points in the jump region may originate from the emergence of singularities during the topological transition, such as monopoles suggested by the magnetic force microscopy image of bulk Fe0.5Co0.5Si29. In addition, several transitions in the interval are also observed. The simulation results suggest these phases are highly relevant to emergence of the elongated skrymion, that is, bimron, the image of which is shown in Supplementary Fig. 5.
For an even thicker NW with a width of 80 nm, the isothermal MR curves display completely different transport behaviour from the narrow NWs, but corroborate the well-established scenario for helimagnets5,17: the helical phase (H) is stable at low fields (B<BS) and then transits into the skyrmion state (S) at BS via a discontinuous phase transition. At even higher fields (B>BC), the conical phase appears and eventually turns into the ferromagnetic ordering above BF. As the NW diameter (d∼80 nm) is much larger than the single skyrmion size (Ld∼18 nm), closely packed skyrmions are hosted, leading to a skyrmion lattice, rather than a skyrmion cluster, and the continuous MR(B) curve between BS and BF. This is in contrast to the jumps in MR seen in narrow NWs due to the emergence of skyrmion clusters.
As a proof, in the other limit when the NW is extremely narrow, the discontinuous jumps indicating the number of skyrmions should be absent. To this end, a NW with a width of ∼20 nm is examined. The MR follows a smooth curve with two transition fields (marked as BS and BC) in the whole magnetic field region (Fig. 5c). This is expected for such narrow NWs because each small triangular NW fails to host a single skymion (with a size of ∼18 nm). These experimental observations are also reproduced by the MC simulation, as shown in Supplementary Fig. 6, where only helical, distorted conical and field-polarized ferromagnetic states exist. However, the calculated transition fields are much smaller than those inferred from the experimental measurements. On the other hand, compared with the thicker NWs, we observed the high critical temperature and magnetic hysteresis behaviour around BS at low temperature. Previous experimental work identified that the critical ordering temperature is strongly affected by finite size effect in NWs16. A similar hysteresis was also observed in the easy-plane B20 MnSi/Si(111) film when the magnetic field is applied along the plane30. These similarities suggest the important role of finite size effects for such ultra-narrow wires. It has been extensively discussed that the change of lattice structure at the crystal boundary or surface contributes an additional magnetic anisotropy or interfacial DM interaction31. Because of the large surface-to-volume ratio in the ultra-narrow NW, we expect these additional interactions to play a significant role in determining the magnetic phases and magnetization process. Nevertheless, based on the MR data and our simple parameter-free model, it is not possible to conclusively decide which magnetic structures are responsible for the field-driven transitions in the MR data. Therefore, based on the numerical results, we only suggest possible helical and distorted conical phases separated by BS. This is also supported by the fact that the MR curve appears to be similar to that observed in bulk MnSi at low temperatures25, where only helical, conical and field-polarized ferromagnetic states exist. Discussions about the additional surface interactions are beyond the scope of this work.
On the basis of the MR data for these NWs at temperatures below Tc (see the detailed data in Supplementary Fig. 4), we can summarize the T–B phase diagrams for NWs with different diameters, as shown in Fig. 5d–f. For d∼20 nm, the critical field BF is much larger than that in bulk MnSi (Fig. 5f). Importantly, as the size of the NW increases, a skyrmion cluster phase emerges. At d∼40 nm, which is about two times larger than Ld, for example, the skyrmion cluster state is dominant while the conical state appears in a tiny T–B window on the negative branches at low temperatures (Fig. 4c). As the NW diameter further increases, individual skyrmions are closely packed into a lattice (Fig. 5d) through a crossover region (Fig. 5e).
We have demonstrated the presence of skyrmion cluster states in confined MnSi NWs with diameters comparable to single-skyrmion domain size. The maximum number of skyrmions within this cluster is determined by the dimension of the NW cross-sections, and the number of skyrmions can be controlled by external magnetic fields and revealed by quantized jumps in the MR curves. These results not only reveal new physics of the skyrmion cluster states in confined geometries, but also can guide the development of skyrmion-based memory devices in which the individual skyrmions could be utilized for multibit memory cells.
All MnSi nanowires (NWs) used in this work were synthesized by chemical vapour deposition using MnCl2 precursor onto silicon substrates14. To fabricate NW devices for magnetotransport measurements, a single NW was picked up from the original silicon substrates and transferred onto a new clean Si substrate coated with 300 nm silicon oxide by three-axis hanging joystick oil hydraulic micromanipulators under an optical microscope, where a home-made tip was used to pick up the NW (See Supplementary Fig. 1). Four Pt or W electrodes were patterned onto an individual NW using focused-ion beam techniques with a small beam current of 7.7 or 24 pA, using a FEI Helios Nanolab 600i. Before Pt deposition, the contact areas were milled by ∼5 nm with a beam current of 1.1 pA to remove surface oxide. To avoid contamination of the electrode and destruction of the sample by the Ga ion source, a 200 nm thick PMMA resist was used to cover the rest of the samples between the electrodes by regular e-beam lithography technique before the fabrication of the electrodes (See Supplementary Fig. 2).
Standard four-probe transport measurements on individual NWs were carried out in a Physical Property Measurement System (Quantum Design Inc.) with a 16 T superconducting magnet. For the transport measurements, to obtain good data with high signal-to-noise ratio, large currents of 30, 10, 5 and 2 μA were used to measure the 80, 55, 40 and 20 nm NWs, respectively. Transport data under small currents were also measured to make sure that the effects of joule heating on the experimental results due to large current density were negligible. All MR(B) data were recorded by increasing B from −8 kOe to 8 kOe. The sweeping fields corresponded to the properties of NWs under field cooling (FC). We also recorded the initial MR curves, reflecting the properties of NWs under zero FC (by cooling the NWs to the defined temperature from far >Tc, for example, ∼50 K, in zero magnetic field before recording the MR data). However, this difference between ZFC and FC does not significantly affect the final results (Supplementary Fig. 7).
To support the experimental observations, MC simulations were performed to get a clear picture of the spin configurations. A generally accepted Hamiltonian for chiral magnets including direct and indirect magnetic coupling with constants A and D, magnetization m, and external field energy is written as29,32
For the MC simulation, the 40 nm NW is divided into two discrete blocks with unit magnetization S, then, a 3D lattice Hamiltionian corresponding to equation (1) is written as
where J denotes the ferromagnetic exchange coupling constant; is DM interaction vector with and is the vector pointing along site i and j; <ij> denotes the nearest spins. Br stands for the reduced magnetic field. The constructed model is schematically illustrated in Supplementary Fig. 8.
In the discrete model, both direct and DM exchange in an inhomogeneous state will have slightly different energy depending on their orientation with respect to the underlying discrete bond orientation of the crystal lattice. Contrary to the isotropic continuous model in equation (1), the discrete model in equation (2) used in the MC simulations leads to the anisotropy energy. To smear out this effect, a corrected term Ec is added as29
where <<ij>> represents the next nearest spins. The ratio D/J was chosen to be consistent with the value adopted in ref. 29, where the wavelengths of d=10 lattice constants were used.
Concerning the real geometry, open and periodic boundary conditions were adopted in the cross-sectional plane of the NW and the long axis, respectively, and a boundary forming the same NW geometry as the experimental merohedral twin plane, which divides the NW into two equal parts with opposite chirality32. Thus, the sign of the coefficient D is opposite in the two domains. According to the previous Lorentz TEM observations in another B20 compounds FeGe, the inversion of the lattice chirality (handedness) of the B20 structure across certain grain boundaries would lead to the invariance of the sign of the spin–orbit interaction within FeGe. It was also observed that the spins around the boundary are almost parallel with the grain boundary. This observation implies that the ferromagnetic interaction would play a dominant role in the narrow transition region where the inversion of the lattice chirality (handedness) occurs, yielding the nearly parallel spin arrangements in the thin region of crystal boundaries33. Thus, the value of D is set to zero in the boundaries20. A high temperature annealing metropolis algorithm is used to obtain the equilibrium spin configurations. At each temperature, the system is allowed to relax towards equilibrium for the first 105 MC steps and thermal averages are calculated over the subsequent 105 steps.
How to cite this article: Du, H. et al. Electrical probing of field-driven cascading quantized transitions of skyrmion cluster states in MnSi nanowires. Nat. Commun. 6:7637 doi: 10.1038/ncomms8637 (2015).
Felser, C. Skyrmions. Angew. Chem. Int. Ed. 52, 1631–1634 (2013).
Mühlbauer, S. et al. Skyrmion lattice in a chiral magnet. Science 323, 915–919 (2009).
Yu, X. Z. et al. Real-space observation of a two-dimensional skyrmion crystal. Nature 465, 901–904 (2010).
Jonietz, F. et al. Spin transfer torques in MnSi at ultralow current densities. Science 330, 1648–1651 (2010).
Rößler, U. K., Leonov, A. A. & Bogdanov, A. N. Chiral Skyrmionic matter in non-centrosymmetric magnets. J. Phys: Conf. Ser. 303, 012105 (2011).
Nagaosa, N. & Tokura, Y. Topological properties and dynamics of magnetic skyrmions. Nat. Nanotechnol. 8, 899–911 (2013).
Iwasaki, J., Mochizuki, M. & Nagaosa, N. Current-induced skyrmion dynamics in constricted geometries. Nat. Nanotechnol. 8, 742–747 (2013).
Sampaio, J. et al. Nucleation, stability and current-induced motion of isolated magnetic skyrmions in nanostructures. Nat. Nanotechnol. 8, 839–844 (2013).
Lin, S. Z., Reichhardt, C. & Saxena, A. Manipulation of skyrmions in nanodisks with a current pulse and skyrmion rectifier. Appl. Phys. Lett. 102, 222405 (2013).
Shibata, K. et al. Towards control of the size and helicity of skyrmions in helimagnetic alloys by spin–orbit coupling. Nat. Nanotechnol. 8, 723–728 (2013).
Iwasaki, J., Mochizuki, M. & Nagaosa, N. Universal current-velocity relation of skyrmion motion in chiral magnets. Nat. Commun. 4, 1463 (2013).
Wilson, M. N. et al. Extended elliptic skyrmion gratings in epitaxial MnSi thin films. Phys. Rev. B 86, 144420 (2013).
Wilson, M. N. et al. Discrete helicoidal states in chiral magnetic thin films. Phys. Rev. B 88, 214420 (2013).
Romming, N. et al. Writing and deleting single magnetic skyrmions. Science 341, 636–639 (2013).
Higgins, J. M., Ding, R. H., DeGrave, J. P. & Jin, S. Signature of helimagnetic ordering in single-crystal MnSi nanowires. Nano Lett. 10, 1605–1610 (2010).
Yu, X. Z. et al. Observation of the magnetic Skyrmion lattice in a MnSi nanowire by Lorentz TEM. Nano Lett. 13, 3755–3759 (2013).
Du, H. F. et al. Highly stable skyrmion state in helimagnetic MnSi nanowires. Nano Lett. 14, 2026–2032 (2014).
Du, H. F. et al. Field-driven evolution of chiral spin textures in a thin helimagnet nanodisk. Phys. Rev. B 87, 014401 (2013).
Leonov, A. O., Rößler, U. K. & Mostovoy, M. Target-skyrmions and skyrmion clusters in nanowires of chiral magnets. EPJ Web Conf. 75, 05002 (2014).
Szczech, J. R. & Jin, S. Epitaxially-hyperbranched FeSi nanowires exhibiting merohedral twinning. J. Mater. Chem. 20, 1375–1382 (2010).
Mena, F. P. et al. Heavy carriers and non-Drude optical conductivity in MnSi. Phys. Rev. B 67, 241101(R) (2003).
Togawa, Y. et al. Interlayer magnetoresistance due to chiral soliton lattice formation in hexagonal chiral magnet CrNb3S6 . Phys. Rev. Lett. 111, 197204 (2013).
Kang, J. & Zang, J. D. Transport theory of metallic B20 helimagnets. Phys. Rev. B 91, 134401 (2015).
Yi, S. D., Onoda, S., Nagaosa, N. & Han, J. H. Skyrmions and anomalous Hall effect in a Dzyaloshinskii–Moriya spiral magnet. Phys. Rev. B 80, 054416 (2009).
Kadowaki, I. K., Okuda, K. & Date, M. Magnetization and magnetoresistance of MnSi. J. Phys. Soc. Jpn. 51, 2433–2438 (1982).
Benjamin, J. C. et al. Large enhancement of emergent magnetic fields in MnSi with impurities and pressure. Phys. Rev. B 88, 214406 (2013).
Meynell, S. A. et al. Surface twist instabilities and skyrmion states in chiral ferromagnets. Phys. Rev. B 90, 014406 (2014).
Huang, S. X. et al. Magnetoresistance due to broken C4 symmetry in cubic B20 chiral magnets. Preprint at http://arxiv.org/abs/1409.7867 (2014).
Milde, P. et al. Unwinding of a skyrmion lattice by magnetic monopoles. Science 340, 1076–1080 (2013).
Karhu, E. A. et al. Chiral modulations and reorientation effects in MnSi thin films. Phys. Rev. B 85, 094429 (2012).
Rößler, U. K. & Bogdanov, A. N. Chiral Symmetry breaking in magnetic thin films and multilayers. Phys. Rev. Lett. 87, 037203 (2001).
Yi, S. D., Onoda, S., Nagaosa, N. & Han, J. H. Skyrmions and anomalous Hall effect in a Dzyaloshinskii-Moriya spiral magnet. Phys. Rev. B 80, 054416 (2009).
Yu, X. Z. et al. Near room-temperature formation of a skyrmion crystal in thin-films of the helimagnet FeGe. Nat. Mater. 10, 106–109 (2011).
This work was supported by the National Key Basic Research of China, under Grant No. 2011CBA00111; the National Nature Science Foundation of China, Grant No. 11174294, No.11474290, No. 11104281, No. 11374302, No. 11222434, No. U1432251; the Anhui Provincial Nature Science Foundation of China, Grant No.1308085QA16; National Basic Research Program of China, Grant No. 2013CB934600; US National Science Foundation, Grant No. ECCS-1231916; US Department of Energy, Grant No. DEFG02-08ER46544; and the Theoretical Interdisciplinary Physics and Astrophysics Center. We thank Weike Wang and Yuyan Han for assistance with the sample measurements by Physical Property Measurement System.
The authors declare no competing financial interests.
About this article
Cite this article
Du, H., Liang, D., Jin, C. et al. Electrical probing of field-driven cascading quantized transitions of skyrmion cluster states in MnSi nanowires. Nat Commun 6, 7637 (2015). https://doi.org/10.1038/ncomms8637
Rare Metals (2022)
Rare Metals (2021)
Scientific Reports (2020)
Journal of Low Temperature Physics (2019)
Nature Nanotechnology (2018)