## Abstract

Low dissipation data processing with spins is one of the promising directions for future information and communication technologies. Despite a significant progress, the available magnonic devices are not broadband yet and have restricted capabilities to redirect spin waves. Here we propose a breakthrough approach to spin wave manipulation in patterned magnetic nanostructures with unmatched characteristics, which exploits a spin wave analogue to edge waves propagating along a water-wall boundary. Using theory, micromagnetic simulations and experiment we investigate spin waves propagating along the edges in magnetic structures, under an in-plane DC magnetic field inclined with respect to the edge. The proposed edge spin waves overcome important challenges faced by previous technologies such as the manipulation of the spin wave propagation direction, and they substantially improve the capability of transmitting information at frequencies exceeding 10 GHz. The concept of the edge spin waves allows to design a broad of logic devices such as splitters, interferometers, or edge spin wave transistors with unprecedented characteristics and a potentially strong impact on information technologies.

## Introduction

Recently there has been an increasing interest in the use of spin waves for information transmission and processing^{1,2,3,4,5,6}. In contrast to spintronics where information is controlled by the relative allignment of ferromagnetic electrodes (see for example ref. 7), here the information encoded in the amplitude and phase of spin waves eliminating the contribution of charge dissipation. As a consequence, spin waves (SWs) propagate coherently through large distances even at room temperature. Contrary to the classic electromagnetic waves, a relatively small group velocity reduces the SWs wavelength down to the nanoscale. This opens new possibilities for a higher integration density in spin-wave logic devices through the effective manipulation of SWs propagating through periodic interferences or arrays of scatterers. The related research field of magnonics has been reviewed recently^{1, 8,9,10}. Gaining an effective control over SWs through their redirection^{11,12,13}, multiplexing^{14} or data processing^{4} is a very active research area nowadays. The global aim is the creation of SW based logic devices.

One of the most important features for future spin wave logics is the broadband capability of its building blocks. Also crucial is SW guidance, including the ability to split spin waves and/or redirect them at large effective angles. So far, the basic building blocks for SW transmission, redirection and control have consisted in straight or curved ferromagnetic strips^{11, 13, 14}. Such elements transmit information via SW modes which have a restricted frequency range (typically below 10 GHz) and are essentially suppressed after changing the direction of propagation up to 90 degrees or by increasing the drive frequency^{11, 13, 14}. This strongly limits the development of redirectional SW logic devices with broadband microwave capabilities.

One way to circumvent the problem is reprogrammable magnonic wave guides made out of dipole interacting elements with controlled switching of their local magnetization^{15}. A fundamentally different approach would be to create low dimensional SW logics with spin waves propagating along artificial or natural magnetic domain walls. Predicted by Winter^{16} SWs propagating along domain walls (DWs) have been identified in a number of recent experimental magnetization configurations in patterned films, involving the domain walls connecting magnetic vortices and edge magnetic charges^{17,18,19,20,21}. The main drawback of the classic DW magnonics is its relatively low frequency of operation and certain difficulties to redirect SWs.

This work explores edge spin waves (E-SWs) propagating along edge domain walls (E-DWs) localized at magnetic nanostructure edges (triangular dot, see Fig. 1) and displaying a number of remarkable and unprecedented features. Besides the broadband character (with the capability to process information at frequencies above 10 GHz) E-SWs (i) can split easily comparing to the conventional spin waves, (ii) could be redirected at angles up to 120 degrees and (iii) show interference phenomena providing the possibility to create phase controlled nanoscale microwave emitters.

The proposed approach based on E-SWs could constitute a fruitful platform for the creation of low dissipation, ultrafast E-SW information processing devices such as spin wave diodes, multiplexors or phase detectors. An effective incorporation of the spin waves in data processing devices requires their transmission and direction control using more complicated structures than just straight or curved micro waveguides - currently among the basic elements of magnonic waveguides^{3, 4}. The capability of changing the SW direction opens perspectives for the creation of novel logic elements based on the SW interference^{13}.

## Results

### Spin wave guidance along the edges

We consider patterned magnetic elements - equilateral triangular magnetic dots with the sides of 2000 nm and thickness 30 nm (Fig. 1b,c). The static bias magnetic field *H*_{
DC
} is directed along the triangle base. This geometry avoids butterfly-type E-DWs which appear when the field is applied perpendicularly to the base of triangle (so-called Y-state) and rectangles (Fig. 2). Previous studies of the edge SWs carried out in rectangular and strip magnetic elements only used in-plane driving RF fields perpendicularly to the applied DC field^{22, 23}. Therefore, increasing the DC field perpendicular to the edge affects E-DW related energy so that mainly inner strip SWs are excited above some critical field^{24, 25}. The internal magnetic field profiles for rectangular elements are shown in Fig. 3.

In contrast to those studies, E-SWs in the triangular dots can be excited using a parallel pumping scheme (with homogeneous driving microwave magnetic field being parallel to the field *H*_{
DC
})^{26} to avoid excitation of the quasi-uniform mode inside the device. Another important differentiating factor is that, as we shall see below, for triangular dots the edge modes could be excited locally, close to the dot edge, facilitating their propagation along the edges.

Indeed, as shown by the dashed lines (cross sections in Fig. 1c), under a DC field parallel to one of their sides, the internal magnetic field distribution has minima near the dot edges which should provide localization of SW at the dot edges. The magnetization dynamics is described by the Landau–Lifshits–Gilbert (LLG) equation of motion governed by an effective magnetic field. SW guidance along E-DWs occurs because the effective field (*H*_{
eff
}) is formed by both the external and the internal magnetic fields, with the latter generated by the volume and surface magnetic charges.

So, increasing the properly aligned DC bias field under excitation localised near vertices just further confines the E-SWs towards the dot edges allowing a continuous field tuning of the E-SW frequency without breaking the SW topology. Our paper presents studies of two related cases: triangular dots in the so-called B state (the bias magnetic field is parallel to the triangle base) and the rectangular dots in the inclined external magnetic field.

### Analytical model for the edge guided spin waves

Below we formulate an approximate analytical model of the localized spin waves which are guided along an edge domain wall in a thin magnetic dot. The main idea is to consider the spin wave propagation in an inhomogeneous potential formed by the dot edge. We start by discussing the similarities and differences between the present model and Winter’s model of SWs localized at the Bloch wall in an infinite ferromagnet^{16}.

Winter^{16} considered 180-degree Bloch DW connecting two semi-infinite oppositely magnetized ferromagnetic domains in an infinite ferromagnet with uniaxial magnetic anisotropy. Firstly, in our case instead of the uniaxial anisotropy constant (*K*) responsible for the domain formation in the Winter model, we have a dot shape anisotropy of magnetostatic origin. The magnetization vector is parallel to the edge plane to minimize the side surface magnetic energy and then, it gradually rotates in the film plane to the direction parallel to the triangle base due to influence of the bias magnetic field applied parallel to the base. It has a maximum magnetization tilting angle of about 60 degrees with respect to the dot edge plane due to the restricted geometry of the dot. In other words, the magnetization inhomogeneity near the dot lateral edges can be described as an incomplete Néel domain wall as sketched in Fig. 1a). The magnetization rotates in the element plane to avoid the face magnetic charges, see Fig. 1b). We consider that the dot edge plane (E-DW) plays a role similar to the DW plane in the Winter model and edge localized SWs propagating along the dot edge in the present case are similar to the Winter magnons propagating in the domain wall plane.

Secondly, in our case the E-DWs are naturally pinned by the element edge, providing (for soft magnetic permalloy patterned nanostructures) a dominant contribution to the additional magnetic anisotropy responsible for this pinning. On the contrary, due to the absence of such a natural edge pinning in the bulk ferromagnet Winter had to introduce an artificial pinning described by the additional magnetic anisotropy *K*′^{16}. The stiffness of the Winter DW being proportional to the anisotropy constant *K*′ is assumed to be much smaller than the E-DW stiffness in triangular dot which is formed by the magnetostatic energy.

The magnetic energy of the dot can be described by the functional:

with the energy density:

where $A$ is the isotropic exchange stiffness constant, ** m** =

**/**

*M**M*

_{ s }is the unit magnetization vector,

*M*

_{ s }is the saturation magnetization,

*H*_{ m }is the magnetostatic field, and

**is external magnetic field (directed along the triangular base).**

*H*Using Eq. (2) we get the dispersion relation for the edge localized spin waves in triangular dots as the following (see Methods):

where *κ* is the spin wave vector along the dot edge, ${l}_{e}=\sqrt{A\mathrm{/2}\pi {M}_{s}^{2}}$ is the exchange length, $h=H/4\pi {M}_{s}$ is the reduced bias magnetic field parallel to the triangle base, and $\nu =\xi {l}_{e}/\sqrt{h}$ is a parameter of the model. The parameter $\nu =\xi /{\xi}_{0}$ is the ratio of the spatial decays of the dynamic (*ξ*) and static (${\xi}_{0}=\sqrt{h}/{l}_{e}$) magnetizations increasing the distance from the dot edge (see Methods). The calculation of the value of *ν* is beyond the present approximate model. We can state only that *ν* < 1 to secure a spin wave frequency increase with *h* increasing. The domain wall considered above is stable in the bias magnetic field *h* > *h*_{
c
}, where the critical field *h*_{
c
} corresponds to transition from the dot vortex state to the B-state increasing the field *h* directed along the triangular dot base. The vortex annihilation field *h*_{
c
} is increasing function of the dot aspect ratio thickness/(in-plane size), *t*/*a*^{27}. This is also confirmed directly with our micromagnetic simulations (Supplementary Fig. 1) which show that relatively small bias fields destabilizing the vortex state in the triangular dot require triangle base size *a* of several micrometers.

The frequency gap *ω*(*κ* = 0) is due to a finite value of the bias magnetic field *h* forming the Néel domain wall. We note that all static and dynamic magnetostatic energies (except the energy of the dot face magnetic charges) were neglected deriving Eq. (3). I.e., the magnetostatics is accounted in a simplified form as a) an “easy plane” magnetic anisotropy forming 2D Néel domain wall near the dot edge; b) as the energy defining the strong pinning boundary conditions for magnetization at the dot lateral edges. Therefore, Eq. (3) is valid within the limit of thin dots, when the dot aspect ratio $t/a\ll 1$.

### Local excitation and control of edge spin waves

In the following we describe results on numerical experiments which support the possibility to excite, redirect and operate E-SWs and to fabricate E-SW magnonics devices. The presence of both surface and point (vertex) magnetic charges allows effective channeling, re-routing and external control of an unprecedented broadband frequency E-SWs.

Based on this fact, one can think of using the edges as transmitters of spin waves, generated at the corners of the triangles. To test this idea we have performed simulations in which a DC film saturates the sample to achieve the B magnetization state (Fig. 1b) and a local AC magnetic field applied only at the base linked vertex of the triangle. The latter generates spin waves that propagate with a considerable amplitude along the dot edges, exceeding the rest of the sample (Fig. 4a and Supplementary video 1). The top corner behaves as a second emitter when the E-SWs reach it, and the waves start propagating along the second “channel”, along the other lateral edge of the dot. The net effect is that waves are transmitted through the corner without reflections and therefore change their direction without any significant loss of intensity. Of course, as they advance through the ferromagnetic material they are damped, and their intensity decays with distance, but the presence of the corner does not yield any additional loss. With this method, E-SW emitted at one corner (for example, at bottom left corner) can reach the opposite corner (bottom right corner), not in a straight line, but through a longer path (bottom left - top - bottom right corner). Then, E-SWs prove that they can be used to overcome a deflection angle of (at least 120°). Our simulations show that the present strategy works also for isosceles triangles.

The right bottom part in Fig. 4a) presents a mechanical model explaining the redirection mechanism behind the E-SWs. Two strings are connected at point through so-called Robin boundary conditions (i.e. mass/massless point fixed by spring) represent E-DWs inter-connected at the upper triangle vertex by the magnetic charge (Fig. 1c). String waves (E-SWs) could be in principle redirected within a large range of angles ($0<\mathrm{\Phi}<\pi $) if two strings are kept tense (i.e. E-DWs are present) and are interconnected through Robin conditions (vertex magnetic charge).

We stress that not all E-SW frequencies are equally valid for being transmitted between the vertices. The spin waves eigenfrequencies are determined by the applied field, which in turn controls the width of the channels. The physical size of the dots is not a factor that affects these eigenfrequencies, as long as we are comparing regions without bends, corners, etc. In the straight sections of the edge, as we shall see further below, only the applied magnetic field affects the wave frequency.

The set consists of around 10 eigenfrequencies that are typically available in the triangular device (Supplementary Fig. 2). Edge SWs with the lowest frequencies “see” a very wide “exchange channel”, while waves with the largest frequencies “see” how it narrows until, eventually, the “channel” is too narrow for the waves to propagate through. We have found that waves with intermediate frequencies show an optimum relation between their wavefront width (too wide wavefronts do not result in waves propagating further than the corner, due to interferences between the incident and deflected waves) and their amplitude to be used in devices. The simulations show that E-SWs are robust to variations of the triangle dimensions between 1 and 2 *μ*m, as well as to the triangle aspect ratio.

The possibility of E-SWs that propagate through the dot corners opens perspectives for creation of a new class of reliable and relatively simple information processing devices. To start with, one can imagine a number of ways to interrupt the E-SW propagation leading to E-SW diode. This could be done, for example by limited rotation of DC magnetic field. Strong sensitivity of the E-SW spectra to the DC field angle allows the interruption of the E-SW propagation through small changes in the DC field angle, as well as to make the spectrum of SWs change.

Another (easier to realize on the small scales) strategy of blocking E-SW propagation from E-SW emitter (*E*) to collector (*C*) could be through injection of spin polarized current to modify locally the damping close to an upper vertex with strongest magnetic charge (base *B*, see sketch in inset of Fig. 4b). High damping should result in an effective blockade of the waves before they turn the upper corner *B*, therefore never reaching the right bottom corner *C*. Figure 4b) shows the simulated transmitted E-SW power when emitted from the bottom left corner to the bottom right corner, passing through the upper one, and with a variable damping *α*_{1} close to *C*. While for the locally suppressed damping the transmitted power is substantially increased for *α*_{1} < *α*_{0} (*α*_{0} is damping of Permalloy). In the opposite limit with ${\alpha}_{0}\simeq 1$ one observes a plateau with even some small increase of the transmitted power caused by bouncing back of the E-SWs without entering to the high damping region.

### Edge spin waves interferometer and splitter

The design of the E-SW interference device based on a single triangular dot is straightforward. For a constructive (or destructive) interference, two in-phase (or in opposition of phase) signals can be sent from the two bottom dot corners producing waves that propagate through their respective “channels”, to end up interfering at the upper corner (Fig. 5 and Supplementary videos 2 and 3). They could be detected, for example, through measurement of the local stray magnetic field near the upper corner. A minimum stray field is observed in the proximity of the upper corner in the conditions for destructive interference. A precise control over the relative phase and amplitude of both emitters opens a wide variety of possibilities in terms of interfering waves.

The nanometer sized stray field tuned by E-SW interference in vertex of a single triangular dot could be used to create near field microwaves (NFM). For example, when in-phase E-SWs are excited in the dot corners (1,3), constructive interference results in the enlarging of the total oscillating local field near point (2) in the an about 10 nm proximity to the vertex. On the other hand, with the out-of-phase interference, one could create extremely localized oscillating magnetic fields in a few nm around corner (2), Fig. 5b). Having gained control over NFM emission in the triangular dot device, one could further explore the NFM capabilities, for example, for effective writing bits with triangles as write heads in the hard disk drives, in substitution of the currently implemented inductive coils.

Since standard SW technology is based on the propagation and detection of SWs through the ferromagnetic strips, we can also consider a E-SW splitter and interferometer based on a strip with two connected by their bases triangles (Fig. 5e). The idea is to use a triangle-like structure in the B state to split effectively spin waves directed from a ferromagnetic strip. Figure 5e) and Supplementary video 4 demonstrate by simulations the effective splitting of spin waves propagating along the strip onto two E-SWs at the intersection between strip and the triangular shape. The proposed E-SW splitter, analogously to the standard optic splitters, allows the realization of an effective interference through backwards transition in the point where opposite strip line situates (see Fig. 5e). We have introduced a slit between two triangles to show that only E-SWs contribute to the backwards interference process.

### Generalization of edge spin waves to magnetic strip

Next we demonstrate that edge spin waves are not specific to magnetic triangular dots only, but could be excited along edges of magnetic rectangular elements (strips) too when a quasi homogeneous DW is created along the device edge. In order to excite spin waves along the edges of a magnetic strip, contrary to the usual practice, the applied magnetic field should not be perpendicular to the strip direction, but tilted at an angle in order to eliminate the possibility of the “butterfly type” interruption in the centre of the exchange energy channels (Fig. 2). For an arbitrary geometry in magnetic nanostructures (as long as they are not too thin, which would force all the magnetization to lay parallel to the edges), an external field which is inclined with respect to the edges results in uninterrupted exchange channels that can be used for propagating spin waves.

Figure 6 summarizes our results on the generation of E-SWs in a 30 nm thick Permalloy strip with lateral dimensions of 1 by 0.5 *μ*m. Our simulations show that for the chosen sample geometry the most homogeneous E-DW appears when an in plane magnetic field is inclined to about 20° with respect to the vertical to the long side of the strip. We also demonstrate effective propagation of broadband E-SWs in rectangular element (Fig. 6b). Finally, Fig. 6c,d) show how the E-DW channel width decreases with the magnitude of inclined DC magnetic field.

### Comparison with between theory, simulations and experiment

In order to excite mainly E-SWs in magnetic substructures one has to create as homogeneous as possible E-DW and predominantly excite the spin waves near DW extremes. We approach these conditions experimentally in the array of magnetostatically decoupled triangular dots and investigate the sample microwave response with microwave field parallel to the applied DC field. In that configuration we both create edge domain wall to channel Winter magnons (Fig. 1) and excite them mainly locally close to vertices.

Our results are shown in Fig. 7, where we compare the measured spectra of an array of 30 nm thick dots (part a) with an array of 100 nm thick dots (part b). All dots are triangular, with a lateral size of 2 *μ*m. The interesting feature of these results is that it is clearly visible how the highest frequency branches are stronger at high fields, and almost invisible at low fields, where the lowest frequency modes are stronger. This confirms the relationship of the width of the exchange channels and E-SW bandwidth with the applied field as observed in simulations and experiment (Fig. 7). Higher frequency waves can only propagate through narrow channels, achieved at high fields. Likewise, the intensity of the low frequency modes becomes weaker at high fields. Another interesting feature (which will be discussed in details elsewhere) is presence of the modes typical for the magnetic vortex state observed at low fields only. As expected, the vortex state exists in a broader field range for 100 nm thick dots in comparison with 30 nm thick dots.

In order to corroborate the main analytical result (equation 3) numerically, we have carried out simulations of the dispersion relation for the E-SWs modes excited by uniform microwave field in an infinitely long strip of 1 nm thickness, (with periodic boundary conditions in the *x* direction, and not in *y*) subjected to an inclined in-plane DC field of magnitude 1000 Oe directed at 60° with respect to the sample face. This has been done because the analytic model considers E-SWs propagating along a semi-infinite plane, within a domain wall without surface magnetic charges. Thicker samples provide a more complicated dispersion curve, with several branches, not accounted by the analytic model, which is valid for very thin samples. Figure 8 compares the E-SW frequencies as a function of the in-plane wave vector obtained numerically, for a 1 nm thick semi-infinite film, since the thickness is small in the analytical model (colored 3D plot), and analytically by using Eq. (3) (line) with only one free parameter of the model tuned (we used *ν* = 0.2, the frequency is weakly dependent on *ν* up to 0.4). Taking into consideration the above discussed applicability limits of the theory, we find the agreement to be satisfactory. We believe that the linear dispersion relation at relatively large *k* is a numerical artifact of the micromagnetic simulations.

### Factors to be considered in real device fabrication

The following factors should be considered during design of E-SW based real devices. Our simulations do not take into account possible influence of the edge related structural disorder. The influence of the structural disorder could be two-fold. First, it could change locally the magnetic damping. The deviation from perfect symmetry of the upper vertex might be important to consider for optimized E-SW transmission between the triangular dot sides. While the above factors would be less important for few micron sized triangles, they should be more carefully considered in nanoscale triangles. One way to circumvent the edge related disorder would be by using self-assembled magnetic triangular dots, such as triangular (111)-oriented LSMO nano-islands^{28}. On the other hand, one has to take into account increases of the bias field needed to propagate E-SWs in smaller size devices. Supplementary Figure 3 demostrates with simulations that triangules of smaller lateral size require stronger bias fields to keep the exchange energy localized near the edges in the B state.

Further studies should also verify the possible influence of coupling to the substrate on E-SWs. One of the routes to improve applicability and functioning of the E-SW based communication devices is fabricating them using YIG films instead of metallic Permalloy, taking advantage of dramatic reduction of the magnetization damping in these insulating ferromagnets. As to the need in application of the external magnetic field, its role in creation of the B-state could be played by exchange bias field with an underlying antiferromagnet. Supplementary Figure 4 shows simulations of the hysteresis loops of a triangular dot placed over a layer of fixed spins, which represent an antiferromagnet. Different exchange couplings between the two layers shift the hysteresis cycle to higher or lower fields, so that the B or Y dot magnetization state could be achieved at zero external field using this method.

## Conclusions and Perspectives

In *Conclusion*, the here proposed edge spin waves could potentially become a unique tool for low dissipation and broadband transmission and processing of information. Their unmatched features allow for effective control and redirection of the spin waves through topologically protected well defined and narrow paths. This concept can be used to design different spin wave logic and sensing elements, such as diodes, multiplexors, read/write heads etc. Also, modulation of the signals could be investigated in more detail in order to produce more complex, non linear devices, logic gates, mixers, etc. Engineering of the shapes of the nanostructures would allow to use edge spin waves to suit different needs, for specific systems of different sizes, configurations, etc. For larger systems, where the waves could be damped out before they reach their final destination, it is important to find materials with low magnetic damping. At present, YIG seems to be the ideal candidate, regardless of some difficulties in its growth and lithography with small size devices, as compared to metallic ferromagnets such as permalloy. Finally, we believe that some of the proposed strategies to develop topologically protected E-SW based communication and signal processing devices could also be implemented in other nanoscale structures. For example, spin-wave edge excitations have been predicted recently in two.dimensional arrays of dipolarly interacting magnetic nanodots^{29, 30} and ferromagnetic spins on a honeycomb lattice with perpendicular anisotropy^{31}.

## Methods

### Experimental set-up

The high-frequency measurements were taken using a network analyzer (VNA), feeding a variable frequency microwave signal to a coplanar waveguide, onto which the sample is placed. The waveguide generates a variable frequency magnetic field which drives the sample. When a resonance frequency is excited, the sample absorbs more energy and we see a decrease in the VNA transmitted signal from the emission port to the detection port. An electromagnet provides the necessary external magnetic field to bias the sample. A computer automatizes the process of fixing a static magnetic field, and sweeping the high frequency, and finally save the spectrum before going to the next static field. For further detail refer to ref. 19.

### Micromagnetic simulations

The micromagnetic simulations were carried out using the OOMMF and Mumax3 codes. The typical magnetic parameters for Permalloy (*Ni*_{80}*Fe*_{20} alloy) were used: saturation magnetization *M*_{
s
} = 830 kA/m, damping constant *α* = 0.01, exchange stiffness $A=1.4\ast {10}^{-11}\phantom{\rule{.1em}{0ex}}\mathrm{J}/\mathrm{m}$. The triangle base size *a* is 2 *μm*, and the dot thickness is *t* = 30 nm or 100 nm. To find the eigenfrequencies of a magnetic structure, a 10^{−3} ns gaussian in-plane magnetic field pulse was applied uniformly. After a 10 ns relaxation time, with the Fourier Transform of *M*_{
x
}(*t*) magnetization component the spin wave eigenmode spectrum is obtained. Knowing the eigenfrequencies, which appear as peaks in the absorption spectrum, a local excitation at a single eigenfrequency can be applied to observe the response of the whole structure (i.e., to observe the propagation of spin waves away from the source), for as long as it may be necessary for the spin waves to reach the target area. To obtain the dispersion relation in Fig. 8, an almost semi-infinite plane (the rectangular sample with periodic boundary conditions in one direction, and a large enough size in the other) is excited with a short field pulse, all the time under the influence of an inclined DC field at 60°. The *z* projection of the magnetization in the simulation cells parallel to the boundary of the sample, and near it (to make sure we are considering waves in the edge domain wall) is saved for different times. With this space vs. time 2D array of data, a Fourier Transform in 2D provides the corresponding wavevector - frequency array, whose amplitude represents the dispersion relation of the waves along the selected path.

### Analytical calculations

To conduct analytic calculations of the edge localized SWs we introduced the coordinate systems, *xyz* and *x*′*yz*′ for description of the magnetization and SW wave vector components. The axis *z* is in the dot plane and perpendicular to the dot edge plane *xOy*, the *x* axis is along the dot edge in the dot plane, and *y* axis is perpendicular to the dot plane (see Fig. 1b). The angle *θ* of the dot in plane static magnetization *M*_{0} changes from zero to 60 degrees. It is convenient to describe magnetization dynamics in the coordinate system related to the *M*_{0} direction denoted as *x*′ axis. In this coordinate system the dynamic magnetization components are *m*_{
z′} and *m*_{
y
}.

The static magnetization *M*_{0} is parallel to the dot edge (the plane *z* = 0), *θ*(0) = 0, due to the side surface magnetostatic energy. Then, the angle *θ*(*z*) increases with the coordinate *z* increasing due to finite bias magnetic field applied parallel to the triangular dot base (a) and forms a Néel like domain wall (Fig. 2). We account that the domain wall localization area is much smaller than the triangle side and consider the domain wall texture far from the triangle corners. We also assume that the triangle dot thickness *t* is much smaller than the equilateral triangle size *a*. This assumption allows us to neglect all magnetostatic energies except the energies related to the face surface magnetic charges accounted as “easy” plane anisotropy, and the side surface charges accounted via the strong pinning boundary conditions at the dot edges. It is convenient to introduce the angle $\phi (z)=\pi /3-\theta (z)$. The static Lagrange-Euler equation for our geometry defining an equilibrium dependence of *ϕ*(*z*) is:

Eq. (4) admits the solution $\mathrm{tan}(\phi (z)/4)=\phantom{\rule{.25em}{0ex}}\mathrm{tan}(\phi \mathrm{(0)}/4){e}^{-\sqrt{h}z/{l}_{e}}$, where $\phi \mathrm{(0)}=\pi /3$. It describes a 60-degree Néel domain wall, where the magnetic field *h* plays a role of the uniaxial magnetic anisotropy responsible for the wall formation.

To consider the magnetization dynamics on the background of the 60-degree Néel domain wall introduced above we use the Landau-Lifshits equation of magnetization motion:

It is convenient to use spherical angles of the magnetization vector $(\mathrm{\Theta},\mathrm{\Phi})$ in the *xyz* coordinate system and write the decomposition $\mathrm{\Theta}={\mathrm{\Theta}}_{0}+\mathit{\vartheta}$, $\mathrm{\Phi}={\mathrm{\Phi}}_{0}+\psi $, where the spherical angles $({\mathrm{\Theta}}_{0}=\pi /2-\theta ,{\mathrm{\Phi}}_{0}=0)$ describe the static domain wall profile and the angles $\mathit{\vartheta}$, $\psi $ describe small deviations from the equilibrium magnetization direction. Then, we search for the solution in the form of plane spin waves propagating along the dot edge, *xOy* plane, $\mathit{\vartheta}(x,z,t)=\mathit{\vartheta}(z,\omega ){e}^{i(\kappa x-\omega t)}$, $\mu (x,z,t)=\mu (z,\omega ){e}^{i(\kappa x-\omega t)}$, where $\mu =-\phantom{\rule{-.25em}{0ex}}\psi \phantom{\rule{.1em}{0ex}}\mathrm{sin}\phantom{\rule{.1em}{0ex}}({\mathrm{\Theta}}_{0})$. Any dependence of the static and dynamic magnetizations on the dot thickness coordinate *y* was neglected assuming thin enough dot. The system of equations of motion for the spin wave profiles $\mathit{\vartheta}(z,\omega )$, *μ*(*z*, *ω*) is the following:

where ${\omega}_{M}=\gamma 4\pi {M}_{s}$, *ϕ*(*z*) is the domain wall profile, and the spatial derivatives are taken with respect to the dimensionless coordinate *z*/*l*_{
e
}.

The function cos *ϕ*(*z*) is a smooth increasing function of *z*, varying from 1/2 to 1 increasing *z*/*l*_{
e
} from 0 to infinity. It describes a potential well for the spin waves traveling along the triangular dot edge. The well exists solely due to finite value of the bias magnetic field *h*. The bottom of the well is located at the dot edge *z* = 0. Increase of the value of the bias field *h* results in decrease of the localization area of the spin waves near the edge *z* = 0. To find an approximate solution of the system of equations (6) and (7) we substitute the variable term *h* cos *ϕ*(*z*) to its spatial average over the distance $l\gg {l}_{e}$, $h\phantom{\rule{.1em}{0ex}}\mathrm{cos}\phantom{\rule{.1em}{0ex}}\phi (z)\to \wedge h\approx h-O({l}_{e}/l)$. Then, we search for the solution of Eqs (6) and (7) in the form of the edge localized spin waves $\mathit{\vartheta}(z,\omega )=\mathit{\vartheta}(\omega ){e}^{-\xi z}$, $\mu (z,\omega )=\mu (\omega ){e}^{-\xi z}$ and get a homogeneous system of equations for the spin wave amplitudes $\mathit{\vartheta}(\omega )$, *μ*(*ω*). Calculating the determinant of this system and equaling it to zero yields the dispersion relation (3) for the spin waves displayed in the main text. The model parameter $1/\xi $ is the length of the decay of the dynamical magnetization components increasing the distance from the dot edge. It can be found from micromagnetic simulations. We simulated (Fig. 4a) that the localization area of dynamical magnetization ($1/\xi $) is about 10–12% of the triangular base size for 2 *μ*m dot with the thickness of 30 nm (i.e., 200–240 nm, essentially larger than the dot thickness). The localization area of the static magnetization ($1/{\xi}_{0}$) is essentially smaller (about of 20–30 nm) and comparable with the the dot thickness. This justifies using the ratio *ν* < 1 in Eq. (3) of the main text (calculated *ν* is 0.09 for the dot thickness 30 nm, *l*_{
e
} = 5.7 nm and the bias magnetic field *H* = 1000 Oe).

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## Acknowledgements

Authors acknowledge José Luis Prieto for the samples fabrication. The work in Madrid has been supported by SVORTEX through CCC-UAM, NVIDIA Academic GPU Grant Program, by Spanish MINECO (MAT2015-66000-P) and the Comunidad de Madrid through NANOFRONTMAG-CM (S2013/MIT-2850) grants. K.G. acknowledges support by IKERBASQUE (the Basque Foundation for Science). The work of K.G. was partially supported by Spanish MINECO grants MAT2013-47078-C2-1-P, FIS2016-78591-C3-3-R, and the European Union’s Horizon 2020 research and innovation program under the Marie Skłodowska-Curie grant No. 644348.

## Author information

### Affiliations

#### Departmento Física Materia Condensada, C03, IFIMAC - Condensed Matter Physics Center and INC- Instituto Nicolas Cabrera, Universidad Autónoma de Madrid, 28049, Madrid, Spain

- Antonio Lara
- , Javier Robledo Moreno
- & Farkhad G. Aliev

#### Departmento Física de Materiales, Universidad del País Vasco, UPV/EHU, 20018, San Sebastián, Spain

- Konstantin Y. Guslienko

#### IKERBASQUE, the Basque Foundation for Science, 48013, Bilbao, Spain

- Konstantin Y. Guslienko

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### Contributions

F.G.A. supervised the project. A.L. performed numerical simulations and experimental measurements with help by J.R.M. The theoretical model was developed by K.G. The paper was written by F.G.A., A.L. and K.G. All authors commented on the paper.

### Competing Interests

The authors declare that they have no competing interests.

### Corresponding author

Correspondence to Farkhad G. Aliev.

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