In the field of magnetism and spintronics chiral magnetic structures, such as spin spirals, domain walls and skyrmions1,2,3,4,5,6, are intensively investigated due to their fascinating properties such as potentially enhanced stability and efficient spin–orbit torque driven dynamics7,8,9,10. It has been shown that these structures are stabilized by the Dzyaloshinskii–Moriya interaction (DMI)11,12 that favors a chiral winding of the magnetization. This antisymmetric indirect exchange interaction requires materials with large spin–orbit coupling as well as a broken inversion symmetry, present in special bulk systems such as B20 compounds where skyrmions have been first discovered experimentally1,2 or in interfacial systems such as heavy metal/ferromagnet multilayer stacks3,4,5,6,8,10. The domain-wall type (Néel or Bloch) and chirality of the spin textures can be accessed in real space by imaging techniques4,13,14,15 or in reciprocal space by (resonant) magnetic X-ray scattering16,17,18. The chiral wall spin structure is of key importance as it governs the dynamical properties of domain walls and skyrmions7,8,9,10,19. While the investigation of static structures and slow (ns) dynamics of chiral magnetic structures has been intensified recently, experimental studies addressing the ultimate fs-ps dynamics of the chirality have been elusive so far. Ultrafast pump-probe experiments have concentrated on the collinear order in magnetic systems20,21,22,23,24,25,26,27,28 with also some studies of non-collinear order in antiferromagnets29,30. In particular, as the ferromagnetic alignment minimizes the Heisenberg exchange energy, while the chiral order results from the DMI, the ultrafast dynamics of both orders needs to be probed individually. Moreover, since the characteristic timescale for the onset of the chiral magnetic order and its ultrafast dynamics are unexplored up to now, we need to ascertain both, as they hold fundamental insights into the underlying physical mechanisms and allow us to gauge the ultimate speed for the manipulation of chiral magnetism, e.g., for ultrafast writing of chiral spin textures.

In this work, we employ circularly polarized light pulses from an extreme ultraviolet (XUV) free-electron laser (FEL) and investigate time-resolved the evolution of the chirality of domain walls in magnetic thin film samples by an IR pump—X-ray magnetic scattering (XRMS) probe experiment.

Using samples with interfacial DMI and perpendicular magnetic anisotropy exhibiting labyrinth-like domain patterns, we measure in the same experiment both the sum signal corresponding to the ferromagnetic order in the domains and the difference signal corresponding to the average chiral order in the domain walls. We find an ultrafast intensity decrease of both signals in the sub-ps regime with similar time constants. However, a significantly faster recovery of the chiral signal in the sub-ns timescale is observed. We subsequently investigate the origin of the faster recovery of the chiral signal by performing numerical simulations of the scattering signal, which reproduce the experimental findings.


Magnetic small angle X-ray scattering

The experimental setup for the scattering experiment is shown schematically in Fig. 1a. Circularly polarized XUV radiation of 60 fs pulse duration was tuned to a wavelength of 23.0 nm corresponding to the Fe M2,3 dichroic transition, which exhibits magnetic scattering contrast due to the X-ray magnetic circular dichroism (XMCD) effect27,28,31,32. The limited transmission in the XUV regime required us to perform the experiment in reflection geometry with an incident angle of Θ = 44°28 yielding an effective XUV penetration depth of ≈8 nm. Owing to an isotropic disordered domain structure we observe the typical ring-like diffraction feature well known from magnetic transmission small angle x-ray scattering (SAXS) experiments representing a broad distribution of Fourier components of the magnetic domain pattern27,28. The sample is pumped with a 60 fs IR laser pulse of 780 nm wavelength impinging on the sample with a small 2 degree offset with respect to the XUV beam (further setup information can be found in the “Methods” section).

Fig. 1: Experimental setup and diffraction images.
figure 1

a Measurement geometry: a magnetic thin film sample is pumped by an optical infrared laser pulse and probed by a circularly polarized X-ray FEL pulse with an incident angle of Θ = 44° (wavevector k, s-polarization (σ) and p-polarization (π)) that scatters on the sample. Afterwards an IR-protected charge-coupled device (CCD) detector records the magnetic SAXS pattern. b MFM image of a typical labyrinth domain pattern of the [Ta(5.3 nm)/Co20Fe60B20(0.93 nm)/Ta(0.08 nm)/MgO(2.0 nm)]x20/Ta(1.6 nm) sample. The inset shows the FFT with the first order peak corresponding to isotropic distributed labyrinthine stripes with a domain periodicity of (455+/−30) nm. These magnetic structures lead to the SAXS signals for left-hand (CL) and right-hand (CR) circular polarized incident X-rays. d The resulting sum =  CL+CR (Eq. (1)) of the diffraction pattern confirms that the diffraction corresponds to the magnetic domains observed by MFM. e The dichroic scattering signal = CL-CR (Eq. (2)) and its azimuthal dependence f confirms the presence of c right-handed chiral Néel (cycloidal) domain walls.

The reflection SAXS pattern was detected on a two-dimensional CCD-detector and investigated as a function of the pump-probe delay over a time span of 100 ps. For each time delay and helicity, 7000 scattering patterns have been measured, normalized to the incoming flux and averaged. The area around the beamstop and charge scattering streaks have been masked. The background from the charge scattering due to the reflection geometry has been subtracted for each pattern, leading to the corrected patterns used in the further analysis.

The investigated [Ta(5.3 nm)/Co20Fe60B20(0.93 nm)/Ta(0.08 nm)/MgO(2.0 nm)]x20/Ta(1.6 nm) multilayer stack was produced by dc magnetron sputtering and exhibits perpendicular magnetic anisotropy (PMA). The material was imaged via magnetic force microscopy (MFM) as shown in Fig. 1b and exhibits, after out-of-plane demagnetization, labyrinth-like magnetic domains at zero field. The domain pattern extended through all ferromagnetic layers due to stray field coupling exhibits a domain periodicity of (455 ± 30) nm. In reciprocal space the MFM images yields a first order peak at q = (13.8 ± 0.9)/μm. Owing to partial alignment of the magnetic stripes, higher order peaks are visible as well33. Further material analysis with a superconducting quantum interference device (SQUID) yields a saturation magnetization of Ms = (844 ± 28) kA/m and an effective perpendicular anisotropy Keff = (133 ± 17) kJ/m3 of the sample at room temperature (for more sample details see “Methods” section). The Ta(5.3 nm)/Co20Fe60B20 interface leads to a positive DMI, with reported values for such stacks ranging from 0.06 to 0.30 mJ/m234,35,36, which favors right-handed Néel-type domain walls (see Fig. 1c). The exact domain-wall arrangement is finally determined by an interplay between interfacial DMI and dipolar interactions, which can lead to complex domain-wall arrangements as shown recently37. We also note that considering the small penetration depth of the XUV radiation, we are sensitive to the magnetization of the topmost Co20Fe60B20 layer only.

X-ray scattering from such magnetic structures leads to the ring shaped SAXS patterns shown in Fig. 1d. We facilitate the discussion by referring to expressions of scattering signals from a one-dimensional magnetic domain arrangement with perpendicular magnetization in the z-direction, lattice spacing d and Neel-type domain walls with a rotation into the x-direction. For this case the sum signal from intensities measured with circular left (CL) and right (CR) polarized light is given by (details see “methods”):

$$I^{{\mathrm{CL}} + {\mathrm{CR}}}(Q) = 2\left| {\mathop {\sum }\limits_n e^{iQdn}} \right|^2\left[ {\left| {m_z(Q)} \right|^2 + \left| {m_x(Q)} \right|^2} \right]$$

with \(m_{z,x}(Q)\) denoting the Fourier transform of the magnetization profiles. The strength of the ICL+CR signal is thus predominantly connected to the average domain magnetization magnitude (I \(\propto\) M2)27,38. Figure 1d displays the corresponding sum image of the CL and CR signals showing a ring-like diffraction pattern at a q-value of (14.3 ± 0.1)/μm that we assign to the 1st order scattering peak of the magnetic stripe domains.

The sensitivity to the chirality of domain walls is obtained via the dichroic (CL-CR) scattering signal:17

$$I^{{\mathrm{CL}} - {\mathrm{CR}}}(Q) = 4\left| {\mathop {\sum }\limits_n e^{iQdn}} \right|^2\left[ {\Im (m_x(Q))\Re (m_z(Q))} \right]$$

the strength of which is given by the correlator \(\Im (m_x(Q))\Re (m_z(Q))\) between z- and x-components of the magnetization. We also note that, in contrast to the CL + CR signal, phase information is preserved in the dichroic signal allowing us to determine the domain-wall chirality (left/right-handed) and character (Bloch (helical), Néel (cycloidal))17,18.

The measured dichroic signal (CL-CR) is shown in Fig. 1e and exhibits a pronounced angular asymmetry with an amplitude of 14 % of the sum signal. Figure 1f shows the orthoradial profile of the dichroic signal. We used a fitting model of A*cos(Ψ − φ), where A is the amplitude, Ψ the azimuthal angle and the phase φ determines the domain-wall angle and with that the domain-wall chirality and character17. Fitting the azimuthal profile leads to a value of φ = 90°, which indeed confirms the predominance of fully right-handed Néel-type domain walls17,18 in the uppermost magnetic layer as expected by micromagnetic simulations of the full material stack in the Supplementary S3. This provides us a tool to individually probe the time-resolved dynamics of the chiral magnetic order in the domain walls.

Ultrafast time-resolved pump-probe experiments

In a next step, we investigated the time evolution of the scattering signals upon IR laser excitation.

Figure 2(a-f) shows the diffraction patterns of the sum and the dichroic signals at different pump-probe delays. At +1.0 ps (Fig. 2b, e)) the intensity in both signals has dropped down significantly in comparison to the initial states (Fig. 2a, d) with a visible partial recovery of both signals after +100 ps (Fig. 2c, f).

Fig. 2: Time dependence of diffraction images.
figure 2

Diffraction patterns for the sum CL + CR (top) and the difference CL − CR (bottom) images for the initial (a, d), +1.0 ps (b, e), and +100 ps (c, f) states. g The experimental (dots) and fitted (lines) orthoradial dichroic profiles for different pump-probe delay times showing a maximum at 90° and a minimum at 270° corresponding to a right-handed cycloidal winding of the domain walls. While the amplitude of the dichroic signal drops within a ps upon pumping and recovers afterwards, no significant angle shift in the fitted phase φ can be detected. The beamstop is located at an azimuthal angle of 90°.

By azimuthal integration of the dichroic signal we can identify that within our experimental accuracy no significant shift in the phase φ of the orthoradial profile (Fig. 2g) has been observed upon pumping. Thereby we can exclude any significant ultrafast change of the domain-wall angle. This means that the DMI is even at the ultrafast timescale contributing to the wall chirality and therewith the stability of chiral spin structures is retained.

The key step is the comparison of the ferromagnetic order dynamics and the chiral order dynamics. To ascertain both, we calculated the average intensity for the sum and the difference signal as a function of the wavevector Qr for different time delays (Fig. 3a, b). The single Qr points shown represent averages of >3000 pixels. Averaging these signals in addition along Qr (radial average) represents averages over 7.1 × 105 pixels containing in total between 1 × 105 and 5 × 105 photons. With this the numerical integration of the radial profiles for each time delay leads to the data shown in Fig. 4a, which demonstrates the evolution of the total intensity of the sum and the difference signal as a function of delay time normalized to the unpumped total intensity. The data shown in Fig. 4b is the result of a second experimental run and represents the average of three scans shown in the Supplementary S9. We discuss the details of errorbar determination in the Supplementary S8 and note here that the maximum error is on the order of 1% for the data in Fig. 4a and 2% for the data shown in Fig. 4b.

Fig. 3: Time dependence of radial scattering intensities.
figure 3

The radial profiles of the sum CL+CR (a) and difference CL-CR (b) signals for selected delay times. Error bars from counting statistic are smaller than the symbol sizes. The visible fluctuations in the profiles are due to speckles originating from the coherent illumination.

Fig. 4: Time dependence of total scattering intensities and second moments.
figure 4

Time evolution of the (a, b) radially integrated intensity from two different experimental runs and (c, d) the 2nd moments of the sum signal (ferromagnetic order) and the difference signal (chiral magnetic order) from the scan shown in a. The solid lines in c, d provide a guide to the eye.

We note that the time constant of the ultrafast decay of the magnetization is similar for both signals (details in Supplementary S7). However, we observe a stronger demagnetization of the CL-CR signal, which drops to (15 ± 1)% at t = 1 ps while the CL + CR signal drops to a value of (20 ± 1)% only (Fig. 4a), similar values can be seen in Fig. 4b. The obtained data in Fig. 4a demonstrates that the CL + CR signal recovers by an amount of (8 ± 2)% from 1 ps to 100 ps while the CL − CR signal recovers in the same time interval by (26 ± 2)%. Similar values for the second experimental run can be seen in Fig. 4b. We used the model reported in Eq. (3) of the “Methods” section to fit the experimental data27. The model includes the time constant τd of the demagnetization process of the ferromagnetic collinear order, respectively, the dechiralisation process (vanishing of the chiral order in the domain walls), and the time constants τr1 and τr2 of the fast and slow recovery processes. The initial ultrafast demagnetization time constant τd = 0.39 ± 0.10 ps is in agreement with the typical demagnetization times of ferromagnetic 3d-transition metals21,22,23,27,28. The main results of these experiments are firstly a dechiralisation process (τd = 0.31 ± 0.10 ps) that occurs on similar timescales as the demagnetization of the collinear domains, and secondly we observe a clear difference in the recovery process of the two signals that occurs on longer timescales. The time constant τr2 = 312 ± 18 ps of the difference signal is significantly smaller than the sum signal (τr2 > 900 ps) demonstrating a faster recovery of the dichroic signal that reflects the chiral magnetic order in the domain walls.

To understand the origin of this difference in the recovery, we next investigate the time evolution of the 2nd moments of the radial distributions as displayed in Fig. 4c, d. The 2nd moments (calculated using Eq. (4) in the Methods section) entail additional information about possible ultrafast changes of the radial distribution widths upon IR excitation. The 2nd moment of the sum signal increases significantly upon pumping within 1 ps, indicating a wider radial distribution and, therefore, we can identify stronger fluctuations, leading to a reduced correlation length of the domain-domain correlation function. After 100 ps it has just recovered partially to its unpumped value. In contrast, the 2nd moment of the difference signal decreases slightly within 1 ps to about 90% after optical excitation but recovers afterwards within a few ps to values around the unpumped value. These differences between the 2nd moments of CL + CR and CL − CR may be understood from the 2nd moments ∆ICL of CL and ∆ICR of CR. Defining ∆I1 = [∆ICL + ∆ICR]/2 and ∆I2 = [∆ICL −  ∆ICR]/2 the 2nd moment of the sum signal is ∆ICL + CR = ∆I1 + ∆I2 ICL − CR/ICL+CR, while the 2nd moment of the difference signal is ∆ICL−CR = ∆I1 + ∆I2 ICL+CR/ICL−CR. In our case ICL−CR/ICL+CR is of the order of 10%. Therefore, ∆ICL+CR is rather insensitive to ∆I2. However, ∆ICL−CR is very sensitive to ∆I2, because it is amplified by the inverse magnetic ratio ICL+CR/ICL−CR. When ∆I2 becomes negative, due to a different broadening of the CL and CR signals, ∆ICL−CR may, therefore, decrease. Additionally, we point out that a simple reduction of the magnetization by a single demagnetization factor everywhere in space reduces both ICL+CR(Q) and ICL-CR(Q) by the same factor.


The experimental results show an ultrafast decrease within the first ps of the total intensity of the sum signal that reflects the conventional collinear magnetic order inside the domains, as well as the dichroic signal that corresponds to the chiral order of the domain walls. Both signals decay on similar timescales, indicating that for the ultrafast initial demagnetization process the order of the magnetization itself does not play a major role in our sample system and thus spin-flip probabilities are similar for both orders.

In order to explain the key finding of the experimentally observed faster recovery of the chiral signal after laser excitation we can envisage two different mechanisms: (1) a change in the size ratio between domain walls and domains caused by an increase of the domain-wall width during the whole investigated time-frame or (2) a faster recovery dynamics of the chiral order within the domain walls compared to the ferromagnetic order in the domains, leading to a faster build-up of the chiral magnetization.

The increase of the domain-wall width as required for mechanism (1) can result from the temperature dependence of the micromagnetic parameters, more precisely the effective anisotropy and the exchange constant, as shown in the Supplementary S4. Since the average domain magnetization is directly proportional to the square root of the total intensity of the sum signal one can estimate the temperature evolution of the spin system (assuming the 3-temperature model21) during the pump-probe experiment using the fitted temperature dependence of the saturation magnetization of the sample (see Supplementary S2). This leads to an increased spin system temperature of (493 ± 22) K at a delay time of 1 ps, where the sample is significantly demagnetized, and an already decreased temperature of (469 ± 13) K at 100 ps. Such a sudden change of the micromagnetic parameters is expected to excite a breathing mode of the domain walls. The breathing mode corresponds to a damped ps-scale oscillation of the width of the domain-wall around the new equilibrium wall width as determined by the temperature-scaled micromagnetic parameters. We estimate the equilibrium wall width at the increased spin system temperature to be 11 nm (see Supplementary S4) in comparison to the equilibrium width of 8 nm at room temperature determined in Supplementary S3. Therefore, we estimate that for our system the wall width oscillates between values of 8 nm and 14 nm due to the sudden change of the micromagnetic parameters. Domain-wall breathing frequencies lie in the range of several GHz. Assuming a breathing frequency of 5 GHz, one-half period of the breathing mode amounts to 100 ps, in which the wall expands by 6 nm from 8 nm to 14 nm.

Mechanism (2) is based on a faster recovery of the chiral order parameter of the system in comparison to the collinear order parameter39,40,41. The chiral order parameter is defined here as the in-plane component of the vector Si × Si+1/|sin θ0| with θ0 denoting the average angle between the neighboring spins Si and Si+1 in the wall39,40,41. The chiral order parameter defined in this way is a pseudo-scalar variable analogous to an Ising spin, which takes values of +1 for right-rotating walls and −1 for left-rotating walls, before the pump pulse arrives.

Between 1 ps and 10 ps the electronic part of the system recovers its ground-state properties to a large extent, while the spin system is still excited with a relatively high-spin temperature of about 490 K, which slowly decays on the scale of 10–1000 ps towards room temperature. It is in this time window that the recovery rate of the chiral order parameter is significantly higher than that of the magnetization. This is based on different temperature dependences of the chiral and scalar order parameters as observed in various spin systems, with the chiral order parameter restoring to its ground-state value faster as the temperature is lowered41. The faster recovery behavior can be traced back to the properties of the chiral order parameter as an essentially Ising type variable39,40,42, which is also the basis of exotic spin states such as chiral spin liquids39,40,43.

In order to check the appropriateness of these two mechanisms for our case, we performed numerical simulations of the scattering signal and evaluated—similar to the experiment—the total intensity and the 2nd moments of the sum and difference signal under the influence of these two mechanisms. We start from an initial labyrinth stripe state shown in Fig. 1b with a domain periodicity of 450 nm and a domain-wall width of 8 nm as estimated in the micromagnetic simulations (Supplementary S3). For mechanism (1) the domain-wall width was altered, while keeping the domain periodicity fixed. Mechanism (2) was implemented by introducing smaller amplitudes of the (transversal) magnetization fluctuations to the domain walls compared to the domains emulating the faster build-up of the chiral order parameter.

In Fig. 5a, we show the simulated total scattering intensities of CL + CR and CL − CR as a function of the domain-wall width. For an estimated maximum increase of the wall width towards 14 nm the signal strength of CL − CR increases to 174%, while the CL + CR increases slightly to 100.8%. The ratio of both signals thus increases by a factor of 1.7, which is considerably larger than the experimental value of ≈1.3 as measured at 100 ps (Fig. 4a, b).

Fig. 5: Numerical calculations of total scattering intensities and second moments.
figure 5

The numerically calculated a, b integrated intensity and c, d 2nd moments of the sum signal (ferromagnetic order) and the difference signal (chiral magnetic order) as a function of the a, c domain-wall width and b, d the transversal magnetization fluctuation strength (cone angle in degrees). The 100% value in a, c corresponds to the room temperature domain-wall width of 8 nm. The dashed lines in b, d correspond to the case of fluctuation in the whole system, while the solid lines correspond to the case of reduced fluctuations within the domain walls.

In Fig. 5b, we show the dependence of the simulated total scattering intensities of CL + CR and CL − CR on the fluctuation tilt angle, which characterizes the strength of the transverse spin fluctuations. The dashed and dotted lines in Fig. 5b correspond to a homogeneous distribution of fluctuations throughout the system, while the solid lines represent the case of reduced fluctuations in the walls, but not in the domains. First, we note that the experimentally observed drop of the intensities to ca 15–20% during the first ps in Fig. 4a) corresponds to a fluctuation tilt angle of ca. 64–68° in Fig. 5b (dashed lines). We assume that during the following 100 ps the fluctuations in the walls reduce faster than in the domains caused by the above discussed temperature (and by that delay time) scaling of the order parameters such that finally the solid lines in Fig. 5b describe the intensities. At 100 ps the value of CL + CR observed in Fig. 4a) is 30% and CL − CR is 41% in good agreement with the numerical intensities at a tilt angle of 60° (solid lines in Fig. 5b).

Figure 5c displays the evolution of the 2nd moment of the scattering peak S(Q) from the simulation as a function of wall width. In contrast to the overall intensity (Fig. 5a) we do not observe significant changes in the second moments on increasing the relevant domain widths between 8 nm and 14 nm.

Fluctuations, however, can change the 2nd moments significantly (Fig. 5d). While the 2nd moments of the CL − CR exhibit a non-monotonous behavior with tilt angle (red and orange lines), the CL + CR signal increases with increasing fluctuations—in good agreement with the experimental findings (Fig. 4d). Therefore, the experimentally observed decrease of the 2nd moments of CL + CR after the first picoseconds can be explained by a reduction of the fluctuation strength with increasing delay time. This also holds true when including a faster reduction of fluctuations in the domain-wall, leading to a faster build-up of the chiral order.

Thus, the findings obtained from the second moments support the presence of the fluctuation mechanism (2). An additional contribution of the breathing mode mechanism (1) to the faster recovery of the total intensity cannot be be ruled out completely, since both mechanisms can in principle explain the observed faster recovery of the total intensity of CL − CR, although mechanism (1) overestimates the corresponding increase significantly. However, the presence of mechanism (1) implicates the necessity of breathing frequencies lower than 5 GHz, since otherwise also a decrease of the domain wall width and accordingly CL − CR should be observed within the 100 ps timeframe, which is not the case. Analytical calculations of the domain-wall oscillation frequency44 using the measured parameters suggest that even the strongly reduced anisotropy values at the high-spin system temperatures after the IR excitation lead to oscillation frequencies in the range of 13–17 GHz. This does not fit the experimental data, that could only be explained by an oscillation of <5 GHz. However, if the breathing mode is strongly damped, it is possible that the domain-wall expands without breathing oscillations from the room temperature width of 8 nm to 11 nm. For an expansion from 8 nm to 11 nm we obtain an increase of the (CL − CR)/(CL + CR) ratio of 1.4, similar to the experimental increase of 1.3.

Therefore, we conclude that the main driver behind our experimental findings is likely mechanism (2), leading to a faster recovery of the chiral order in the domain walls in comparison to the ferromagnetic order in the domains. The responsible mechanism(s) might in addition be also material system dependent. So for the future, one can explore further multilayer stacks and the time dependence of the total intensity on even longer timescales to probe if one can identify additionally the effects of a damped breathing mode of the domain-wall excited by the IR laser.

In conclusion, using resonant magnetic scattering at an XUV-FEL we identify a faster recovery of the scattering intensity signal stemming from the chiral magnetic order in the domain walls compared to the signal from the collinear magnetic order in the domains. We also observe an increase of the width of the structure factor peak for the collinear signal while the chiral scattering peak does not increase in width upon IR pumping indicating strong fluctuations. We explain both observations with the onset of strong transversal magnetic fluctuations after pumping in the domain systems. Importantly, however, our experimental findings imply reduced fluctuations within the chiral domain walls, leading to a chiral order that is restored faster. We can connect this to the realization that the characteristic timescale for the onset of the chiral magnetic order is significantly lower than the onset of the ferromagnetic order. In the future further fundamental aspects can be studied in detail, e.g., the dependence of the timescales of the chiral order build-up on the absolute strength of the DMI by varying the heavy metal layers. The control of the DMI and the chirality of spin structures on the ultrafast timescale can finally allow the controlled ultrafast manipulation of chiral magnetism, e.g., ultrafast writing of chiral topological objects such as skyrmions and pave the path to applications in the field of ultrafast chiral spintronics.


Sample fabrication and characterization

The magnetic multilayer sample has been grown at room temperature by dc magnetron sputtering and consist of (thicknesses in nm) Si/SiO2/[Ta(5.3)/Co20Fe60B20(0.93)/Ta(0.08)/MgO(2.0)]x20 /Ta(1.6). The Ta(0.08 nm) interlayer was inserted to tune the anisotropy stemming from the Co20Fe60B20/MgO interface, while the 1.6 nm Ta capping was reduced to a thickness that prevented the sample from oxidation, but simultaneously led to sufficient penetration of the XUV light into the topmost Co20Fe60B20 layer to ensure sufficient statistics. The magnetic properties of the sample were characterized using superconducting quantum interference magnetometry (SQUID) in the temperature range 10 K to 390 K and a vibrating sample magnetometer (VSM) in the temperature range 300 K to 600 K. Both out-of-plane and in-plane hysteresis loops were measured (see Supplementary S1) for each temperature. From those the saturation magnetization Ms and the effective perpendicular anisotropy constant Keff were determined. The latter was ascertained from the difference in the areas of the in-plane and out-of plane loops45. This leads to the temperature dependencies shown in Supplementary S1 yielding a Curie temperature of (553 ± 1) K and parameters Ms(300 K) = (844 ± 28) kA/m and Keff(300 K) = (133 ± 17) kJ/m3 at room temperature. Additionally, a 20 ×20 μm2 MFM image of the multilayers was performed at room temperature as shown in Fig. 1b. The sample exhibits labyrinth-like stripe domains with a domain periodicity of (455 ± 30) nm, as extracted from the Fourier spectrum, which exhibits a first order peak at q = (13.8 ± 0.9)/μm (see Supplementary S5). The interfacial DMI arises from the Ta(5.3 nm)/Co20Fe60B20 interface, which favors right-handed chiral Néel domain walls, as observed in the dichroic SAXS signal in Fig. 1e, f. One must take into consideration that the Ta(0.08 nm) insertion layer is not even a complete Ta monolayer and, therefore, a net interfacial DMI is still prominent in the sample. Finally, the interplay between interfacial DMI and dipolar interactions determines the equilibrium domain and domain-wall arrangement in the sample37 as revealed in the micromagnetic simulations of the full materials stack shown in Supplementary S3.

Pump-probe experiments

The measurements have been performed at the DiProI beamline46,47 at the FERMI FEL facility in Trieste, Italy48,49. For the experiment, the FEL was tuned to the Fe M2,3-edge at a wavelength of 23.0 nm, a pulse duration of 60 fs, a repetition rate of 50 Hz, and an attenuated pulse energy of 0.94 μJ. Using a Kirkpatrick–Baez (KB) optics, the beam was focused down to a size of (200) × (200) μm2, leading to an energy density of 3.0 mJ/cm2. The optical laser for pump-probe experiments is the same as the Ti:sapphire seed laser used for generating the FEL pulses in the HGHG scheme and, therefore, is intrinsically synchronized to the XUV-FEL pulses with a jitter of <10 fs. We used as a pump a 780 nm IR pulse of 100 fs duration, with an energy of 2.62 μJ and a size of (300) × (300) μm2, leading to a pump energy density of 3.7 mJ/cm2, well below the material damage threshold and the intra-pulse self-demagnetization process observed with FEL radiation on similar magnetic structures50. The IR and FEL beams are nearly parallel with a small angular offset of 2°, which allows for a constant temporal resolution during the rotation of the sample through the beam. The resonant magnetic XUV reflectivity experiments were performed for left- and right-hand circular polarization with a charge-coupled device (CCD) area detector (2048 × 2048 pixels, 13.5 × 13.5 µm2 pixel size) placed 145 mm behind the sample. The circularly polarized incident X-rays hit the sample at an angle of 44 degrees yielding an effective penetration depth of 8 nm. The intense reflected primary beam is blocked by a beamstop. The CCD is IR protected by an Al filter. Additional data obtained during the second experimental run and shown in Fig. 4b were measured at three different positions on the sample, under similar experimental conditions. The energy densities were about 3.8 mJ/cm2 for pump (IR laser) beam and 2.0 mJ/cm2 for probe (FEL) beam.

SAXS data treatment

For each measured pump probe time delay, 7000 SAXS patterns have been measured for each helicity. The patterns have been normalized to the incoming flux and averaged. The area around the beamstop and charge scattering streaks along the reflectivity ridge have been masked (white areas in Fig. 2b–2g) leaving 7.1 × 105 pixel for the magnetic scattering analysis. To remove the contribution of the charge component, the background signal is calculated for each pattern. Using the areas inside and outside the diffraction ring, we can reconstruct the whole pattern without the magnetic part. As a result of the background removal, we obtain the corrected patterns for post-proceeding analysis.

Afterwards the average intensity of the sum (CL + CR) and difference (CL − CR) diffraction images was determined as a function of the wavevector Qr for different time delays as depicted in Fig. 3. The radial profiles for each time delay were then integrated in order to obtain the evolution of the total intensity of the sum and the difference signal as a function of delay time. The time evolution of the total intensity normalized to the unpumped total intensity is displayed in Fig. 4a, b.

The time dependence of the total intensities was fitted with the sum of three exponential functions convolved with a Gaussian distribution containing the time resolution σt of the experiment given by the pulse duration of the FEL:

$$I\left( t \right)/I_{{\mathrm{unpumped}}} = \ \left\{ 1 - H\left( t - t_{0} \right) \cdot \left[ A_{d} \cdot {\mathrm{exp}}\left( { - \frac{{t - t_{0}}}{{\tau _d}}} \right) + A_{r1} \cdot {\mathrm{exp}}\left( { - \frac{{t - t_0}}{{\tau _{r1}}}} \right) \right.\right.\\ + A_{r2} \cdot \left.\left. {\mathrm{exp}}\left( - \frac{{t - t_0}}{{\tau _{r2}}} \right) \right] \right\} \ast \left[ \frac{1}{{\sqrt {2\pi } \sigma _t}} \cdot {\mathrm{exp}}\left( - \frac{{\left( {t - t_0} \right)^2}}{{2\sigma _t^2}} \right) \right],$$

where τd denotes the time constant of the demagnetization, respectively, the dechiralisation process and τr1 and τr2 the time constants of the fast and slow recovery processes, whereas Ad, Ar1, and Ar2 denote the strength of these processes (fit parameters displayed in Supplementary S6). H(t) is the Heaviside step function and time zero t0 was obtained from the fit.

The 2nd moments of scattering peak S(Q) (radial scattering distribution) displayed in Fig. 4c, d are calculated by:

$$2{\mathrm{nd}}\,{\mathrm{moment}} = \frac{{\smallint (q - q_0)^2S(q)dq}}{{\smallint S(q)dq}}$$

where the peak center q0 is determined for each delay time individually.

Numerical calculation of the diffracted intensity

In the simulation setup we assume a system of homochiral walls, where the components of the magnetization profiles of the −+ and +− walls are expressed by:

$$m_x^{W - + }\left( x \right) = - m_x^{W + - }\left( x \right) = - \sqrt {1 - [\tanh \frac{x}{w}]^2} \\ m_y^{W - + }\left( x \right) = m_y^{W + - }\left( x \right) = 0\\ m_z^{W - + }\left( x \right) = - m_z^{W + - }\left( x \right) = \tanh \frac{x}{w},$$

with w being the domain-wall width.

In a system of perfectly arranged parallel homochiral domain walls with domain wall periodicity d the magnetization in the magnetic unit cell (from −d/2 to d/2) is given by:

$${\boldsymbol{m}}\left( x \right) = \left\{ {\begin{array}{*{20}{c}} {{\boldsymbol{m}}^{W + - }\left( {x + \frac{d}{4}} \right)for - \frac{d}{2} < x < 0} \\ {{\boldsymbol{m}}^{W - + }\left( {x - \frac{d}{4}} \right)for + \frac{d}{2} > x > 0.} \end{array}} \right.$$

The scattering amplitude resulting from n unit cells is given by:

$$F\left( Q \right) = \mathop {\sum }\limits_n e^{iQdn}(\hat {\boldsymbol{\varepsilon }} \times {{\hat{\boldsymbol\varepsilon}}}^{\prime} )\cdot \int_{ - d/2}^{d/2} {\boldsymbol{m}}(x)e^{iQx}dx,$$

where \({\hat{\varepsilon}}\) and \({{\hat{\boldsymbol\varepsilon}}}^{\prime}\) are the polarization vectors of the incident and scattered beam, respectively.

The form factor of the magnetic domains is given by the integral:

$${\boldsymbol{m}}\left( Q \right) = \, \int_{ - \frac{d}{2}}^{\frac{d}{2}} {\boldsymbol{m}}\left( x \right)e^{iQx}dx \\ = \, 2i\sin \left( {Qd/4} \right)\int_{ - d/4}^{d/4} {\boldsymbol{m}}^{W - + }\left( x \right)e^{iQx}dx$$

and is evaluated numerically. For circular polarized light of handedness λ the scattering intensity is:

$$I\left( {Q,\lambda } \right) = \left| {\mathop {\sum }\limits_n e^{iQdn}} \right|^2\left| {m_x\left( Q \right) + \lambda im_z\left( Q \right)} \right|^2 \\ = \left| {\mathop {\sum }\limits_n e^{iQdn}} \right|^2\left\{ {\left| {m_x\left( Q \right)} \right|^2 + \left| {m_z\left( Q \right)} \right|^2 + 2\lambda \left[ {\Im m_x\left( Q \right)\Re m_z\left( Q \right) - \Re m_x\left( Q \right)\Im m_z\left( Q \right)} \right]} \right\}$$

The difference between the CL and CR intensities is given by:

$$I^{CL - CR}\left( Q \right) = 4\left| {\mathop {\sum }\limits_n e^{iQdn}} \right|^2\left[ {\Im m_x\left( Q \right)\Re f_z\left( Q \right) - \Re m_x\left( Q \right)\Im m_z\left( Q \right)} \right] \\ = 4\left| {\mathop {\sum }\limits_n e^{iQdn}} \right|^2\Im m_x\left( Q \right)\Re m_z\left( Q \right)$$

while the sum of the CL and CR intensities is given by:

$$I^{CL + CR}\left( Q \right) = 2\left| {\mathop {\sum }\limits_n e^{iQdn}} \right|^2\left[ {\left| {m_x\left( Q \right)} \right|^2 + \left| {m_z\left( Q \right)} \right|^2} \right].$$

When including fluctuations we model the diffracted intensity that leads to the data shown in Fig. 5b,  d numerically by calculating numerically the integrated intensity:

$$I\left( Q \right) = |(\varepsilon \times \varepsilon^\prime )\cdot \int _{ - L/2}^{L/2} {\boldsymbol{m}}(x)e^{iQx}dx|^2,$$

where L is the size of the simulation box. We used L = 200 µm, corresponding to 444 domain periodicities of 450 nm. The magnetization m(x) in the system without fluctuations is obtained by alternating −+ and +− walls spaced 225 nm apart. The data shown in Fig. 5 is obtained by averaging over 100 random domain patterns.

In order to model the effect of transverse fluctuations we first tilt the magnetization at every point by a polar tilt angle. After that we rotate the magnetization at every point by an azimuthal angle obtained from a random number generator. We characterize the fluctuation strength by the polar tilt angle.

In order to model the case where fluctuations are reduced in the walls (due to the proposed faster recovery of the chiral order parameter), we switch off the fluctuations in the region \(- 1.1w < x - x_i < 1.1w\) for every wall i.