Abstract
A fundamental property of particles and antiparticles (such as electrons and positrons, respectively) is their ability to annihilate one another. A similar behaviour is predicted for magnetic solitons^{1}—localized spin textures that can be distinguished by their topological index Q. Theoretically, magnetic topological solitons with opposite values of Q, such as skyrmions^{2} and their antiparticles (namely, antiskyrmions), are expected to be able to continuously merge and annihilate^{3}. However, experimental verification of such particle–antiparticle pair production and annihilation processes has been lacking. Here we report the creation and annihilation of skyrmion–antiskyrmion pairs in an exceptionally thin film of the cubic chiral magnet of B20type FeGe observed using transmission electron microscopy. Our observations are highly reproducible and are fully consistent with micromagnetic simulations. Our findings provide a new platform for the fundamental studies of particles and antiparticles based on magnetic solids and open new perspectives for practical applications of thin films of isotropic chiral magnets.
Main
The stability of magnetic skyrmions in B20type crystals results from competition between Heisenberg exchange and chiral Dzyaloshinskii–Moriya interaction (DMI)^{4,5}. Since cubic anisotropy in such crystals is typically negligibly small and, to a first approximation, Heisenberg exchange and DMI are assumed to be isotropic, it is common to refer to them as isotropic chiral magnets. In such systems, DMI is predicted to favour skyrmion solutions of fixed chirality^{6}, in agreement with experimental observations^{7,8,9,10}.
Skyrmions in isotropic chiral magnets typically take the form of vortexlike tubes or strings, which penetrate through the entire sample thickness. As a result of conical modulations, a cross section of an isolated skyrmion tube resembles a twodimensional (2D) skyrmion in a tilted ferromagnetic vacuum^{11}. Recent theoretical studies^{3,12} of a 2D model of an isotropic chiral magnet have revealed many intriguing effects. In particular, it was shown that there is a stable solution for a skyrmion antiparticle—an antiskyrmion—which is characterized by opposite chirality in different spatial directions^{3}.
We begin by checking the stability of such a solution for a film of finite thickness with a threedimensional (3D) model, taking into account demagnetizing fields. Figure 1a illustrates statically stable solutions for a skyrmion, an antiskyrmion, a skyrmionium and a representative skyrmion–antiskyrmion pair obtained by micromagnetic calculations (Methods and Extended Data Fig. 1a,b) (for illustrative purposes, the different spin textures are combined in a single simulated domain in an optimal field at which all of them are stable). The 3D spin textures are visualized by means of isosurfaces and a standard colour code for spin directions. It is important to note that the isolated antiskyrmion and skyrmion–antiskyrmion pair (Fig. 1) are statically stable states and are therefore fundamentally different from the dynamic antiskyrmions that have been discussed earlier^{13,14,15}.
The colour variation at the edges of the simulation box indicates the presence of a conical spiral in the direction of external magnetic field B_{ext} ∥ e_{z}. The period of cone modulations, that is, \({L}_{{{{\rm{D}}}}}=4\uppi {{{\mathcal{A}}}}/{{{\mathcal{D}}}}\), depends on the ratio between exchange stiffness constant \({{{\mathcal{A}}}}\) and DMI constant \({{{\mathcal{D}}}}\). It, therefore, varies between different compounds. For example, in FeGe, L_{D} = 70 nm. As a result of the presence of conical modulations, demagnetizing fields and chiral surface twist, the spin texture notably changes through the film thickness (Fig. 1b). Figure 1c–e shows the simulations of Lorentz transmission electron microscopy (TEM) images and an electron holographic phaseshift image. Supplementary Fig. 1 shows a series of Lorentz TEM images simulated for different defocus distances.
Following a general approach for the classification of solutions in systems in which the order parameter is the unitvector field, the localized magnetic textures (Fig. 1) can be classified based on the topological index as
where m(r) is the magnetization unitvector field. Since the magnetic texture (Fig. 1) is smooth and free of Bloch points, the above definition of Q is valid in any arbitrarily chosen x–y plane. The total topological index of the combined spin texture (Fig. 1) is zero, since the topological indices of a skyrmion and antiskyrmion are −1 and +1, respectively, whereas the topological index of a skyrmionium is zero.
In our micromagnetic simulations, the isolated skyrmion and antiskyrmion remain stable over a wide range of fields, whereas in the pure 2D case, the isolated antiskyrmion stability range is very narrow^{3}. The wide range of antiskyrmion stability in the 3D case can be explained by the gain in DMI energy due to chiral modulations across the plate thickness (Extended Data Fig. 1c,d). The stability of 3D antiskyrmions is also supported by Monte Carlo simulations performed at finite temperatures (Supplementary Video 1) and stochastic Landau–Lifshitz–Gilbert simulations (Supplementary Data 1). In contrast, the skyrmion–antiskyrmion pair (Fig. 1) has weaker stability and annihilates with increasing magnetic field or under the influence of weak perturbations (Supplementary Figs. 2 and 3 and Supplementary Video 2 show details of pair nucleation and annihilation processes). Since skyrmion–antiskyrmion pair annihilation can be triggered in different ways depending on their mutual orientation and environment, strictly speaking, there are no exact critical fields bounding the stability of the skyrmion–antiskyrmion pair. Such behaviour of the skyrmion–antiskyrmion pair is consistent with the prediction of the 2D model, suggesting that on a qualitative level, a 2D model of a chiral magnet is able to capture the main features of a more advanced 3D model. For instance, similar to the 2D case^{3}, the 3D skyrmion–antiskyrmion pair has a few mutual orientations of the skyrmion and antiskyrmion at which they remain stable (Extended Data Fig. 3e shows another stable skyrmion–antiskyrmion pair orientation). The asymmetric interaction potential between the skyrmion and antiskyrmion and the different stability ranges are the fundamental properties that distinguish them from ordinary particles and antiparticles. Below, we provide experimental images of such pairs and compare them with micromagnetic simulations. In particular, we present experimental results on the creation and annihilation of a skyrmion–antiskyrmion pair, which are guided by a different theoretical prediction of a 2D model, which shows that a set of closed domain walls, such as a skyrmion bag, can decay into ‘elementary’ particles—skyrmions and antiskyrmions—in a certain external magnetic field. This decay conserves the total topological index and thus represents a homotopic transition. Extended Data Fig. 2 illustrates such a decay induced by a tilted magnetic field for a skyrmion bag with Q = 1 and skyrmionium with Q = 0 for the 2D model. We find that in a 3D model of a sample with finite thickness, this instability occurs even in a perpendicular applied field.
Micromagnetic simulations of this process in a film of finite thickness in the presence of a demagnetizing field are provided in Extended Data Fig. 3 and Supplementary Fig. 3. Starting with a complex magnetic configuration in zero field, we observe the same qualitative evolution with an applied field as for the 2D case, eventually leading to the formation of skyrmions and antiskyrmions.
To perform experimental observations of the theoretically predicted phenomena, a thin plate was prepared from a single crystal of B20type FeGe using a focusedionbeam workstation and a liftout method^{16}. As shown in the scanning electron microscopy images (Extended Data Fig. 4) as well as the Lorentz TEM images presented below, the sample is defect free and has nearly the same thickness over the whole area. The nominal thickness of the square plate t is comparable to the size of chiral modulations L_{D} (70 nm) in this compound. It should be noted that such an exceptionally thin and uniform film of a B20type chiral magnet has not been studied before, to the best of our knowledge, using Lorentz TEM or other microscopy techniques. Taking into account possible errors in the thickness estimation of ~5 nm and the likely presence of a thin damaged surface layer of ~5 nm due to sample preparation^{17}, it is reasonable to assume that the true magnetic thickness of the FeGe plate is ~50 nm.
Figure 2 shows representative experimental overfocused Lorentz TEM images of a square 1 μm × 1 μm plate of the FeGe sample recorded after distinct cycles of applied external fields. Figure 2a shows a representative ground state of the system in zero field, whereas Fig. 2b–f shows the typical contrast in an external magnetic field of above 200 mT applied perpendicular to the plate. Further experimental images are provided in Extended Data Fig. 6. Note that the pairs shown in Fig. 2c,e are prior states to the skyrmion–antiskyrmion pair depicted in Fig. 1. Theoretical Lorentz TEM images obtained using micromagnetic simulations for skyrmion–antiskyrmion pair nucleation are shown in Extended Data Fig. 3. Excellent agreement is obtained between the theoretical (Fig. 1 and Extended Data Fig. 3) and experimental (Fig. 2) Lorentz TEM images, confirming the formation of the four distinct states shown in Fig. 1. In the overfocused regime, an ordinary skyrmion is imaged as a bright circular spot, whereas an antiskyrmion is imaged as an elongated dark spot with weak bright contrast on only one side. The magnetic contrast of an antiskyrmion in our isotropic case differs from that of an antiskyrmion in a system with anisotropic DMI^{18,19}, as a result of the asymmetry of antiskyrmions and additional modulations through the film thickness. The situation is different for Heusler materials^{18,19}, in which antiskyrmions have a fixed orientation to the crystallographic axes. In contrast, in isotropic chiral magnets, an antiskyrmion has an additional rotational degree of freedom. Antiskyrmions with different orientations are shown in Fig. 2b–f. Since the antiskyrmion orientation is coupled to the inplane components of the external field and remanent magnetization, all the antiskyrmions in the sample are identically oriented (Extended Data Fig. 3e,f). A skyrmionium is imaged as a bright circular halo surrounding a dark spot, whereas a skyrmion–antiskyrmion pair (Fig. 2b,c,e) shows a superposition of skyrmion and antiskyrmion contrast. The TEM images allow a skyrmionium and a skyrmion–antiskyrmion pair (Fig. 2c) to be distinguished despite their topological equivalence. Extended Data Fig. 7 shows the representative underfocused and overfocused Lorentz TEM images as well as the phaseshift images recorded using offaxis electron holography. The comparison between theoretical and experimental phaseshift images shows good quantitative agreement. Supplementary Fig. 6 shows the experimental images of antiskyrmions recorded at different specimen temperatures.
Figure 2g shows the experimentally estimated collapse fields of skyrmions and antiskyrmions as a function of temperature. The trend line of the experimental points for the antiskyrmion collapse field, extrapolated to zero temperature, shows reasonable agreement with the value of ~400 mT provided by micromagnetic simulations (Supplementary Fig. 2). At a magnetic field of ~200 mT (blue circles), weak contrast associated with surfaceinduced modulations^{20,21,22} emerges. This contrast transforms into helical spirals when the field is reduced, making it difficult to estimate the lower bound field for antiskyrmion stability, which is indicated by a blurred lower edge of the magenta region (Fig. 2g).
The experimental images shown in Fig. 2 and Extended Data Figs. 6 and 7 were obtained by using the following approach, which allows the observed magnetic states to be reproducibly generated. First, a perpendicular field of B_{ext} ≈ 50 mT was cycled several times until a pattern of closed domain walls was observed, similar to that shown in Fig. 3a, in which the contour lines marked in white, red and yellow follow 180° domain walls. As a result of the presence of Fresnel fringes from the sample edges, the yellow contours near the left, right and lower edges of the sample only become evident with increasing field (Fig. 3b–e). The white and yellow contours enclose areas in which the magnetization is opposite to B_{ext}, whereas the red contours enclose areas in which the magnetization is along B_{ext}. In Fig. 3, the external magnetic field points towards the reader.
When the external magnetic field is increased, the white contours converge to form skyrmions, whereas the red contours converge to form antiskyrmions (Fig. 3a). The larger the number of red contours present in the initial state, the more antiskyrmions are observed with increasing field, and vice versa. Extended Data Figs. 8 and 10 illustrate antiskyrmion nucleation for different initial states. If the helical modulations in the initial state do not form closed loops, then either only skyrmions or no skyrmions are observed with increasing field. The outer domain walls (Fig. 3a, yellow) typically do not form closed loops and are instead often connected to the sample edges. For example, eight stripes are connected to the upper edge of the sample (Fig. 3a). Our observations show that such stripes may give rise to an arbitrary number of skyrmions. In the present case (Fig. 3), these stripes continuously disappear (Fig. 3g) and the outer domain wall converges to form a single skyrmion. This process can be followed based on the total number of antiskyrmions present at higher magnetic fields (Fig. 3i,j). At intermediate fields, annihilation of skyrmion–antiskyrmion pairs is observed (Fig. 3g,h and Extended Data Figs. 8–10). Representative examples of individual skyrmion–antiskyrmion pair annihilation are presented in Fig. 4.
The weaker stability of skyrmion–antiskyrmion pairs is in good agreement with micromagnetic simulations (Supplementary Fig. 2). Furthermore, theoretical calculations suggest that the particle–antiparticle pair illustrated in Fig. 1 is statically stable only above a critical film thickness, which we estimate for FeGe to be 40 ± 5 nm. In a thinner film, such pairs annihilate immediately, similar to the behaviour for the 2D model (Extended Data Fig. 2). Direct observation of the annihilation process using TEM demands ultrafast imaging with at least nanosecond temporal resolution^{23}.
Despite the topological equivalence between a skyrmion–antiskyrmion pair and a skyrmionium, we did not experimentally observe the transition between the two states. However, micromagnetic simulations suggest that such a transition can be achieved by slightly tilting the magnetic field by several degrees. In contrast to the formation of skyrmion–antiskyrmion pairs, the appearance of a skyrmionium in our experiments was a very rare event. The protocol (recently proposed elsewhere^{24}) provides a reliable approach for the nucleation of a skyrmionium and other skyrmions with topological charge Q ≥ 0.
It should be noted that the approach described above for antiskyrmion nucleation is only applicable for thin plates, for which t ≲ L_{D}. As reported in many earlier works, in thick plates of cubic chiral magnets, irrespective of their initial state, the system usually only converges to an energetically more favourable state that contains skyrmions. An alternative approach for the creation of antiskyrmions in thick plates will be presented elsewhere.
In conclusion, we have observed the creation and annihilation of skyrmion antiparticles in an isotropic chiral magnet—B20type FeGe. Micromagnetic simulations support these observations and show excellent agreement with the experimental data. The experimental observation of skyrmion–antiskyrmion pairs in an FeGe plate whose thickness is below the size of characteristic chiral modulation may serve as a platform to study the fundamental physics of topological solitons in magnetic solids. The good qualitative agreement of the observed phenomena with theoretical predictions for a 2D model^{3} suggests that a large diversity of other phenomena predicted by this model^{25,26,27} may be experimentally verified in thin films of cubic chiral magnets. Our results suggest that a thin plate of an isotropic chiral magnet may provide a platform for the experimental verification of the effect of a sign change in a topological Hall signal when the system contains antiskyrmions instead of skyrmions^{28}. Moreover, they open a wide vista for the experimental study of intriguing phenomena that manifest themselves as additional contributions to a Hall signal, even when the averaged topological density is zero (examples shown elsewhere^{29,30}) for an identical number of particles and antiparticles.
Methods
Micromagnetic calculations
The micromagnetic approach was followed in this work. The total energy of the system includes the exchange energy, DMI energy, Zeeman energy and selfenergy of the demagnetizing field^{31}:
where the magnetic field is
m(r) = M(r)/M_{s} is a unitvector field that defines the direction of magnetization, M_{s} = ∣M(r)∣ is the saturation magnetization, A_{d}(r) is the component of magnetic vector potential induced by the magnetization, \({{{\mathcal{A}}}}\) is the exchange stiffness constant, \({{{\mathcal{D}}}}\) is the constant of isotropic bulk DMI and μ_{0} is the vacuum permeability (μ_{0} ≈ 1.256 μN A^{−2}). In our simulations, we used the following material parameters for FeGe (ref. ^{32}): \({{{\mathcal{A}}}}\) = 4.75 pJ m^{−1}, \({{{\mathcal{D}}}}\) = 0.853 mJ m^{−2} and M_{s} = 384 kA m^{−1}. These parameters provide the period of helical modulations at zero field, that is, \({L}_{{{{\rm{D}}}}}=4\uppi {{{\mathcal{A}}}}/{{{\mathcal{D}}}}\) = 70 nm, and the saturation field for the cone phase, that is, B_{c} = B_{D} + μ_{0}M_{s} = 0.682 T, where \({B}_{{{{\rm{D}}}}}={{{\mathcal{D}}}}/(2{M}_{{{{\rm{s}}}}}{{{\mathcal{A}}}})\) = 0.199 T. Details of the critical field are provided in another work^{33}. The solutions of the Hamiltonian in equation (2) were found by using the numerical energy minimization method^{33} using the Excalibur software^{34}. The termination criterion for convergence was chosen according to the Gill–Murray–Wright method^{35,36} with a function tolerance τ_{F} = 10^{−10}.
Initial guesses for calculating antiparticles
Defining angle ϕ_{A} = πz/L_{D}, the orientation of an antiskyrmion is first set in every z section in the form:
Following the approach introduced elsewhere^{12}, the auxiliary vector field is defined according to the expression
where \({g}_{\pm }=\frac{5}{4}\left({\left({x}^{\prime}\right)}^{2}+{\left({y}^{\prime}\right)}^{2}\right)2{x}^{\prime}{y}^{\prime}\pm 1\) and scaling parameter l defines the antiskyrmion size. In our simulations, we let l = 0.25L_{D}. For an antiskyrmion embedded in a ferromagnetic background, we use the following initial guess:
where R_{z}(ϕ_{A}) is a 3 × 3 rotational matrix about the z axis. For an antiskyrmion embedded in the conical phase, the initial guess takes the form
where θ_{c} is the cone phase angle and ϕ_{c} = 2πz/L_{D}.
An alternative approach for the construction of the initial state for an antiskyrmion is illustrated in Extended Data Fig. 1. This approach has been verified using the Mumax^{37} software.
Magnetic imaging using TEM
Fresnel defocus Lorentz TEM imaging and offaxis electron holography were performed using an FEI Titan 60300 TEM instrument operated at 300 kV. The microscope was operated in aberrationcorrected Lorentz mode with the sample in magneticfieldfree conditions. A conventional microscope objective lens was then used to apply outofplane magnetic fields to the sample, ranging between –0.15 and +1.50 T (precalibrated using a Hall probe). A liquidnitrogencooled specimen holder (Gatan model 636) was used to control the specimen temperature between 95 and 380 K. Images were recorded when the specimen temperature was 95 K, if not specified otherwise. Fresnel defocus Lorentz TEM images and offaxis electron holograms were recorded using a 4k × 4k Gatan K2 IS direct electroncounting detector. The defocus distance was ∣Δz∣ = 800 μm for all the images presented in the text, if not specified otherwise. Multiple offaxis electron holograms, each with a 4 s exposure time, were recorded to improve the signaltonoise ratio and analysed using a standard fast Fourier transform algorithm in HoloWorks software (Gatan).
Theoretical Lorentz TEM and phaseshift images were calculated for numerical micromagnetic solutions by the method described elsewhere^{33} and implemented in the Excalibur software^{34}.
Data availability
Raw data presented in the main text are available at https://doi.org/10.5281/zenodo.5930353. All other data are available from the corresponding authors upon reasonable request.
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Acknowledgements
We thank H. Du for help with the sample preparation. This project has received funding from the European Research Council under the European Union’s Horizon 2020 Research and Innovation Programme (grant no. 856538—Project ‘3D MAGiC’). F.N.R. was supported by Swedish Research Council grants 64220137837, 201606122 and 201803659, and by the Göran Gustafsson Foundation for Research in Natural Sciences. V.M.K. and N.S.K. acknowledge financial support from the Deutsche Forschungsgemeinschaft through SPP 2137 ‘Skyrmionics’ grant no. KI 2078/11. S.B. acknowledges financial support from the Deutsche Forschungsgemeinschaft through SPP 2137 ‘Skyrmionics’ grant no. BL 444/16. R.E.D.B. is grateful for financial support from the European Research Council under the European Union’s Horizon 2020 Research and Innovation Programme (grant no. 823717—project ‘ESTEEM3’; grant no. 766970—project ‘QSORT’) and Deutsche Forschungsgemeinschaft (Project ID 405553726; TRR 270).
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Open access funding provided by Forschungszentrum Jülich GmbH.
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F.Z. and N.S.K. conceived the project and designed the experiments. F.Z. performed the TEM experiments and data analysis together with N.S.K. and L.Y. N.S.K., V.M.K. and F.N.R. developed the theory and performed the numerical simulations. F.Z. and N.S.K. prepared the manuscript. All the authors discussed the results and contributed to the final manuscript.
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Extended data
Extended Data Fig. 1 Antiskyrmion in micromagnetic simulations.
a, Initial state comprising two coaxial cylindrical domains with their magnetization up (white) and down (black), embedded in a conical state whose k vector is 2π/L_{D} and points along the z axis. The cone angle \({\vartheta }_{{{{\rm{c}}}}}={{{\rm{acos}}}}({B}_{{{{\rm{ext}}}}}/({B}_{{{{\rm{D}}}}}+{\mu }_{0}{M}_{{{{\rm{s}}}}}))\). b, Antiskyrmion in an external field of B_{ext} = 0.45(B_{D} + μ_{0}M_{s}) ≈ 300 mT obtained after full energy minimization in Mumax assuming periodic boundary conditions in the xy plane. The 3D spin texture of the antiskyrmion is visualized, showing cuboids at the edges of the simulated domain and cuboids, where m_{z} < 0. The size of the domain in the xy plane is 4L_{D} × 4L_{D} and the thickness is 1L_{D}. For other parameters, see Methods and Supplementary Data 1 with a corresponding Mumax script. c Inplane component of the DMI energy density ω_{DMI}(xy) in the xy plane around the antiskyrmion for different crosssections. Similar to the 2D case^{26}, ω_{DMI}(xy) becomes positive in certain regions. Note that we use the notation ∇_{xy} × n = \(\hat{\bf{i}}\)(− ∂_{y}n_{z}) + \(\hat{\bf{j}}\)(∂_{x}n_{z}) + \(\hat{\bf{k}}\)(∂_{x}n_{y} − ∂_{y}n_{x}), where ∂_{α}n_{β} = ∂n_{β}/∂α. d Distribution of the total DMI energy density ω_{DMI}, which includes both inplane and outofplane components. Because of the chiral modulations along the z axis, the total DMI energy density becomes negative everywhere, even in regions where ω_{DMI}(xy) > 0. The DMI energy gain provides an additional stability to the antiskyrmion in the 3D case. The color bar on the right is identical for both energy densities.
Extended Data Fig. 2 Homotopical transition of a 2D skyrmion bag with Q = 1 and skyrmionium with Q = 0.
a, Stability diagram for the 2D skyrmion bag depicted in b, given in terms of the inplane and outofplane components of the reduced external magnetic field h = B_{ext}/B_{D}. The calculations were performed for a large domain of size 8L_{D} × 8L_{D} (mesh density 64 nodes per L_{D}) for the model Hamiltonian given in Ref. ^{3}. The stability region of the skyrmion bag is bounded by the collapse field from above, the elliptic instability field from below, and the instability with respect to a homotopical (continuous) transition into another state with conservation of the topological index Q on the right. For a magnetic field below h_{e}, the bag becomes unstable with respect to stretching and tends to occupy the whole space of the simulated domain. The spin textures depicted in b and c correspond to stable configurations in different fields (see corresponding labels in a). Contour lines C_{1} − C_{3} indicate closed 180^{∘} domain walls. The yellow contour encloses the area with m_{z} < 0 (black), while the red contours enclose the area with m_{z} > 0 (white)  as in Fig. 2. Images df illustrate the homotopical transition that the skyrmion bag in c undergoes as soon as the external magnetic field exceeds the critical field h_{t} (see the red transition line in a). Images de are unstable configurations, representing snapshots taken at different stages during direct energy minimization, while the antiskyrmion in f is a stable configuration. The antiskyrmion has its own collapse field and elliptic instability field, which are not shown in a. gl illustrate homotopical transition for the skyrmionium depicted in h, which continuously converges to the tilted ferromagnetic state (l) under a homotopical transition via the formation of a skyrmionantiskyrmion pair (j), followed by its annihilation (k).
Extended Data Fig. 3 Nucleation of skyrmionantiskyrmion pairs in 3D micromagnetic simulations.
Each image ad shows the magnetization vector field represented by isosurfaces m_{z} = 0 and corresponding overfocus Lorentz TEM images calculated for defocus distance of 800 μm at different external magnetic fields applied perpendicular to the film. The images in ac illustrate the nucleation of the skyrmion antiskyrmion pair, while de shows other possible configurations. The initial state in a is similar to skyrmionium configuration in Fig. 2b. The infield evolution ac of the magnetization state illustrates the topological transition similar to that observed in the 2D model. d shows the pair after reducing the field back to 200 mT and illustrates the hysteretic effect. e shows another possible orientation of the skyrmionantiskyrmion pair which was experimentally observed, see Fig. 2b and Extended Data Fig. 5. f shows a coupled pair of two antiskyrmions (see for example experimental image in Fig. 2d) and illustrates that the antiskyrmion orientation is coupled to the inplane component of remanent magnetization of the surrounding state. In e and f the direction of the inplane component of remanent magnetization is depicted by the white arrow, m_{r}.
Extended Data Fig. 4 Scanning electron microscopy images of the sample.
a and b show the side and the top view of the sample, respectively. The sample was titled away slightly (by ~ 2^{∘}) from the [110] zone axis.
Extended Data Fig. 5 Comparison of experimental and theoretical Lorentz TEM images of a stable skyrmionantiskyrmion pair at 200 mT at different defocus distances.
a and b show experimental and theoretical Lorentz TEM images in overfocus and underfocus regimes, respectively. The size of the simulated domain and the mesh density are identical to those in Fig. 1 in the main text. The contamination seen on the upper edge of the sample is due to sample degradation. These images were recorded 6 months after all other images. The images were recorded at a specimen temperature of 95 K.
Extended Data Fig. 6 Lorentz TEM images showing contrast features that correspond to a skyrmion, an antiskyrmion, a skyrmionantiskyrmion pair and a skyrmionium.
ae and h show antiskyrmions. f and h show skyrmioniums. c, d, e and g show skyrmionantiskyrmion pairs. The defocus distance is 800 μm. The images were recorded at a specimen temperature of 95 K.
Extended Data Fig. 7 Quantitative comparison between experimental and theoretical images.
a, Representative Lorentz TEM and phase shift images showing contrast features that correspond to a skyrmion, an antiskyrmion and a skyrmionantiskyrmion pair. b, Lorentz TEM and phase shift images of a theoreticallysimulated antiskyrmion. See simulation details in Fig. 1. From left to right: Under, overfocus Lorentz TEM and electron phase shift images recorded using offaxis electron holography. c shows the corresponding magnetization vector field represented by isosurfaces m_{z} = 0 of the antiskyrmion shown in b. d, Line plot profiles of the phase shift of the antiskyrmions shown in a and b at the positions marked by dashed lines. The experimental and theoretical phase shifts are in good agreement. The applied magnetic field in each case is 165 mT. The defocus distance is 600 μm. The images were recorded at a specimen temperature of 95 K.
Extended Data Fig. 8 Lorentz TEM images showing the nucleation of magnetic antiskyrmions.
The initial state of the system was different from that presented in Fig. 3a. The images were recorded overfocus in increasing perpendicular magnetic fields. The magnitude of the field is indicated above each image. a and b are identical. Lines in a mark domain walls, similar to those in Fig. 3a. Red circles mark antiskyrmions, which collapse at 224 mT (see h and i). The two skyrmions labeled in h annihilate with two antiskyrmions with increasing field (see j). j shows a skyrmionantiskyrmion pair, which annihilates with increasing field at 243 mT (see k). The antiskyrmions collapse at a field of 259 mT (see l). The defocus distance is 600 μm.
Extended Data Fig. 9 Lorentz TEM images showing the nucleation of magnetic antiskyrmions.
The initial state of the system has one closed domain wall, which is marked by a red contour and converges to a single antiskyrmion with increasing field. The two white contours converge to two skyrmions with increasing field. The skyrmion and antiskyrmion marked in e annihilate with each other when the field is increased to 208 mT (see f).
Extended Data Fig. 10 Lorentz TEM images showing the nucleation of magnetic antiskyrmions.
The initial state of the system has no closed domain walls that converge to form skyrmions with increasing field. hk show skyrmionantiskyrmion pairs, which annihilate with each other with increasing field (compare i and j, k and l).
Supplementary information
Supplementary Information
Supplementary Figs. 1–6.
Supplementary Video 1
Monte Carlo simulations showing the stability of an antiskyrmion in the presence of thermal fluctuations were performed for a spin–lattice model of a cubic helimagnet. We used the same model and visualization technique mentioned elsewhere^{38}. The simulations were performed on a lattice with 256 × 256 × 64 spins, with periodic boundary conditions in the film plane. The demagnetizing field effect was omitted from this simulation. The DMI and Heisenberg exchange were chosen so that L_{D} ≈ 2πaJ/D ≈ 62.8a, where a is the lattice constant and J = 1 and D = 0.1 are the exchange constant and DMI constant, respectively. The perpendicular magnetic field B_{ext} = 0.7B_{D}. The temperature in the simulation was set to T = 0.33T_{c}.
Supplementary Video 2
Landau–Lifshitz–Gilbert simulations showing annihilation of the skyrmion–antiskyrmion pair induced by the tilt of the external magnetic field from the z axis towards the y axis. Representative snapshots of the video are shown in Supplementary Fig. 3.
Supplementary Data 1
Mumax script for micromagnetic simulations.
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Zheng, F., Kiselev, N.S., Yang, L. et al. Skyrmion–antiskyrmion pair creation and annihilation in a cubic chiral magnet. Nat. Phys. 18, 863–868 (2022). https://doi.org/10.1038/s41567022016384
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DOI: https://doi.org/10.1038/s41567022016384
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