new science opportunities
Hard Xray nanofocusing at lowemittance synchrotron radiation sources
^{a}Institut für Strukturphysik, Technische Universität Dresden, 01062 Dresden, Germany, ^{b}Deutsches ElektronenSynchrotron DESY, Notkestrasse 85, 22607 Hamburg, Germany, and ^{c}Fachbereich Physik, Universität Hamburg, Luruper Chaussee 149, 22761 Hamburg, Germany
^{*}Correspondence email: schroer@xraylens.de
Xray scanning microscopy relies on intensive nanobeams generated by imaging a highly brilliant synchrotron radiation source onto the sample with a nanofocusing Xray optic. Here, using a Gaussian model for the central cone of an undulator source, the nanobeam generated by refractive Xray lenses is modeled in terms of size,
and coherence. The beam properties are expressed in terms of the emittances of the storage ring and the lateral sizes of the electron beam. Optimal source parameters are calculated to obtain efficient and diffractionlimited nanofocusing. With decreasing emittance, the usable fraction of the beam for diffractionlimited nanofocusing experiments can be increased by more than two orders of magnitude compared with modern storage ring sources. For a diffractionlimited storage ring, nearly the whole beam can be focused, making these sources highly attractive for Xray scanning microscopy.Keywords: Xray nanofocus; Xray optics; diffractionlimited storage ring.
1. Introduction
Hard Xray scanning microscopy enjoys an increasing demand in many fields of science, such as physics and chemistry, biology, materials, earth and environmental science, and nanotechnology (Xu et al., 2013: Vogt & Lanzirotti, 2013). Its key strength lies in the large of hard Xrays that can penetrate specialized sample environments, such as chemical reactors, microfluidic or pressure cells. Xray microscopy is thus ideally suited for in situ and in operando studies of physical and chemical processes. By using various Xray analytical techniques as contrast, such as absorption or diffraction, Xray scanning microscopy allows one to measure quantitatively the elemental composition, the chemical state or the local mesoscopic or atomic structure, respectively. In combination with tomography the threedimensional inner structure of a specimen can be reconstructed.
In scanning microscopy, the signaltonoise ratio and the minimal exposure time are limited by the λ ≃ 1 Å) and thus the largest fraction of the beam cannot be used for nanofocusing. Modern synchrotron radiation sources are thus highly inefficient for Xray scanning microscopy, yet still by far the best sources available today.
in the probe beam. Therefore, it requires an intensive Xray nanobeam. In order to achieve highest spatial resolutions, the Xrays from the source are imaged onto the sample in a diffractionlimited geometry. The beam size is then approximately given by the size of the Airy disc and the mainly depends on the of the source and the transmission and numerical aperture of the optic. Diffractionlimited focusing is realised by matching the aperture of the nanofocusing optic to the lateral coherence length of the Xrays falling onto its aperture. This implies that only the coherent fraction of the Xray beam can be efficiently focused. For modern synchrotron radiation sources, the coherent fraction of the beam lies in the range of per mille for hard Xrays (The important figureofmerit of the source is the spectral i.e. per source size, solid angle and energy bandwidth. At fixed power of the source, the optimal is obtained when the source size and solid angle of emission are minimal. This is the case when the source is diffractionlimited, i.e. the source size and divergence match the intrinsic divergence of undulator radiation (cf. §2.1). Today's synchrotron radiation sources have very different beam properties in the vertical and horizontal direction. While in the vertical direction the diffraction limit is reached in many cases even for hard Xrays, the horizontal source size and divergence is much larger than the diffraction limit. The larger horizontal emittance (cf. §2.1) can in principle be reduced by optimizing the electron optics in the storage ring, making the electron beam less divergent and confining it laterally to a smaller area. The Xray microscopist's dream would be a diffractionlimited storage ring (DLSR), where also the horizontal beam size and divergence would match the intrinsic divergence of the undulator radiation.
which describes the Xray that is emitted by the source per phase space volume,In this article we investigate the nanobeam properties, such as beam size,
and coherence, in terms of the source parameters. This can be done analytically within a Gaussian model. For a given undulator source, the optimal storage ring parameters are calculated to optimize the source for scanning microscopy. We show that a reduction in source emittance significantly improves the efficiency of nanofocusing and that ultimately, for a DLSR, the nanofocusing efficiency could be increased by more than two orders of magnitude compared with what is possible today.2. Xray scanning microscope
Xray scanning microscopes rely on a laterally small probe beam that is generated by imaging the source onto the sample in a strongly demagnifying geometry. The nanobeam properties are determined by the relation of the effective aperture of the nanofocusing optic to the beam size, wavefront curvature and lateral coherence length at its entrance. In many cases, scanning microscopes make use of a secondary source to optimally match the abovementioned quantities to each other. Here, for the simplicity of the presentation, we will consider a simpler imaging scheme, imaging the source directly onto the sample by one nanofocusing optic (cf. Fig. 1).
We model monochromatic Xrays as a scalar wavefield that propagates according to the Helmholtz equation (Born & Wolf, 1999). This assumes that polarization effects can be neglected. In a straight focusing geometry (Fig. 1) and considering maximal deflection angles in the range of several milliradians, the paraxial approximation is well justified and the polarization can indeed be neglected. In the following, we model the radiation in the central cone of an undulator source by a Gaussian ensemble of Gaussian limited waves (§2.1). We then propagate this Gaussian ensemble to the refractive lens (§2.2), model the lens in terms of a thin object (§2.3) and propagate the Xrays to an arbitrary distance behind the lens, in particular into the focal plane (§2.4). Minimal focus sizes are obtained in a socalled diffractionlimited imaging geometry that is discussed in §2.5.
2.1. Gaussian model for an undulator source
In the undulator of a synchrotron radiation source the electrons radiate independently of each other and in an uncorrelated fashion. The radiation emitted by an electron is strongly directed into the forward direction by the relativistic aberration and interference of the emission amplitudes for the different poles of the undulator. The resulting rootmeansquare (r.m.s.) opening angle of the emission cone is (Thompson et al., 2009)
where γ is the electron energy relative to its rest mass, κ is the undulator parameter, j is the integer number describing the harmonic of the radiation, and N_{u} is the number of undulator periods. The most important parameters and quantities considered in this article are listed for quick reference in Table 1. The spectrum of the undulator radiation on the optical axis is concentrated in odd harmonics,
with λ being the wavelength of the Xrays, the undulator period, and θ the emission angle relative to the undulator axis.
To model the emission of a single electron at a transverse position and moving into a certain direction relative to the optical axis, the electromagnetic wavefield of the Xrays in the undulator can be described by a complex scalar amplitude,
where is the transverse wavenumber defining the propagation direction of the electron in terms of photon momentum components (q_{x}/k, q_{y}/k) with k = . A_{0} is the amplitude and σ the r.m.s. diffractionlimited source size for the synchrotron radiation emitted by one electron. The Gaussian model for undulator radiation is only valid in the farfield of the undulator, i.e. at distances that are much larger than the length of the undulator. Two exemplary electrons and their emission cones are shown in Fig. 2.
In the storage ring the electrons are confined into bunches, filling a certain region of phase space. In the transverse direction the distribution of electrons can be modeled by a Gaussian ensemble that is defined by the electron density in lateral space and momentum, given by
where and are the r.m.s. source size and divergence in the horizontal and vertical direction, respectively (cf. Fig. 2). If the dynamics of the electrons in the storage ring decouple in the horizontal and vertical direction, the respective emittances : = are constants of motion around the storage ring.
For the purposes of this article, we can describe the radiation from the ensemble of electrons by the mutual intensity function (Born & Wolf, 1999)
that describes the timeaveraged correlation between the field amplitudes at the transverse positions and .
Due to the symmetry of the Gaussian model and the source the mutual intensity function can be separated into the product of two functions that describe the horizontal and vertical beam properties, respectively,
Inserting (2) and (3) into (4), we obtain
and an analogous expression for J_{0v}(y_{1}, y_{2}). I_{0} is the maximal intensity in the source plane. Here,
Equation (6) can be interpreted in the following way: for x = x_{1} = x_{2} the mutual intensity yields the intensity of the wavefield at the location x. The convolution of the Gaussian emission cone with the Gaussian electron density distribution yields an r.m.s. source size of (cf. Fig. 2)
The second exponential term in (6) describes an of the amplitude–amplitude correlation with increasing distance = x_{1}x_{2} in the source. l_{0h,v} is the characteristic correlation length and is called the lateral coherence length in the given direction. It is a function of both the source size and the electron beam divergence.
The source is considered diffractionlimited when and . Making use of the relation between σ and in (2) a diffractionlimited emittance fulfills the following condition (Thompson et al., 2009),
In the diffractionlimited case [, in (7) and (8)], the lateral coherence length l_{0h,v} in the source exceeds the source size by at least 15%. For current synchrotron radiation sources, however, l_{0h,v} is much smaller than the source size (cf. Fig. 2).
2.2. Propagation of the Xrays to the nanofocusing optic
Equation (6) has the Gaussian structure of a socalled Gaussian shell model (Vartanyants & Singer, 2010; Singer & Vartanyants, 2014). This model has been analyzed in detail by I. Vartanyants and A. Singer, including the focusing of a partially coherent beam by refractive Xray lenses (Singer & Vartanyants, 2014). Here, we calculate the mutual intensity function in analogy to Singer & Vartanyants (2014), expressing the results in terms of the source parameters described in the previous section. It is useful to follow the propagation of the beam once again to identify the important parameters and their dependence on the source.
In a first step, the mutual intensity in the source plane given by (6) is propagated to the entrance of the focusing optic located at a distance L_{1} from the source (Born & Wolf, 1999),
where is the Fresnel propagator of the Xrays along the optical axis. In the paraxial Fresnel–Kirchhoff approximation it is given by
The integral (9) can be separated into a product of a horizontal and vertical contribution that, again, can be treated separately in the following.
The horizontal contribution is
A similar expression is found for the vertical direction. As opposed to the wavefield in the source plane, the mutual intensity at a distance L_{1} from the source includes an additional phase term that describes the wavefront curvature. The wavefront is curved with a curvature radius that describes the effective source distance,
that is slightly shorter than the geometric distance L_{1} from the source to the optic and can be slightly different for the horizontal and vertical direction, introducing a slight astigmatism in that case. For current sources, however, the effect is so small that it is not easily observable and can be neglected.
The r.m.s. beam size for the intensity just before the nanofocusing optic (Fig. 1) is
It can be easily interpreted as the width of the convolution of the single electron emission cone with the spatial and angular distribution of the source ensemble defined by equation (3). The products are called the transverse emittances of the photon beam. The of the source is inversely proportional to both these transverse emittances (Thompson et al., 2009). The lateral coherence length is
While L_{1h,v}^{*} determines the position of the focal spot along the optical axis, and l_{ch,v} determine the transmission through the optic and the beam size in the focus. These three quantities fully determine the focal properties. and l_{ch,v} are shown in Fig. 1.
2.3. Focusing by parabolic refractive Xray lenses
There are many different nanofocusing Xray optics available today, exploiting reflection (Jarre et al., 2005; Mimura et al., 2007), diffraction (Chu et al., 2008; Kang et al., 2008; Mimura et al., 2010; VilaComamala et al., 2011; Yan et al., 2011) and refraction (Schroer et al., 2005, 2011, 2013). Nanofocusing refractive Xray lenses are used in the scanning microscopes at beamline ID13 of the ESRF, and beamline P06 of PETRA III (Schroer et al., 2010). For the purpose of this article, it is useful to consider these refractive Xray optics, as their aperture function is intrinsically Gaussian.
Parabolic refractive Xray lenses and their imaging properties were previously described in detail (Lengeler et al., 1999; Kohn, 2003; Schroer et al., 2013). In the case of nanofocusing, they can typically not be considered as thin optics. However, their particular imaging properties (Kohn, 2003; Schroer et al., 2013) allow one to replace the thick optic with an effective Gaussian thinobject transmission model in the case of nanofocusing, i.e. when the sourcetolens distance L_{1} is much larger than the focal length.
In general, the aperture of the nanofocusing optic acts like a spatial filter, truncating part of the electromagnetic wave in the plane of the optic. For a thin refractive focusing optic with focal length f, the transmission function is given by
where is a (potentially complex) aperture function of the optic. For parabolic refractive Xray lenses that are free of aberrations, is real and given by
inside the geometric aperture radius R_{0} and zero outside (Lengeler et al., 1999). T_{0} is the transmission of the Xray lenses on the optical axis and can be minimized by reducing the distance d between the apices of the parabolae (Lengeler et al., 1999). The properties of the lens material enter in equations (14) and (15) implicitly via f and μ.
Here, we consider the case where R_{0} is sufficiently large to justify a fully Gaussian aperture [cf. Schroer et al. (2013) for examples of nearly Gaussian nanobeams generated by refractive nanofocusing lenses]. In this case, the aperture is limited by Gaussian absorption inside the lens material. N is the number of single lenses and R the radius of curvature of an individual lens surface (Lengeler et al., 1999). The effective aperture is defined as (Lengeler et al., 1999)
and describes the value of the width of the transmission of the amplitudes (not intensities) through the lens (Lengeler et al., 1999) and is thus times larger than the r.m.s. width of the intensity transmission profile of the lens.
2.4. Propagating the Xrays through the caustic of the nanobeam
The mutual intensity at the distance L_{2} after the lens is given by
and by symmetry of the problem can again be separated into a horizontal and vertical contribution [cf. (5)]. An arbitrary distance L_{2} behind the optic the horizontal part of the mutual intensity is
The vertical part J_{L2v}(y_{1}, y_{2}) has the same structure. The first exponential term in (18) describes the lateral beam size. The r.m.s. beam size is
where
describes the defocus and
is the effective aperture corrected for the inhomogeneous Gaussian illumination with the r.m.s. width .
The second exponential in (18) describes the wavefront curvature with a curvature radius
The last exponential term in (18) describes the average amplitude–amplitude correlation with a lateral coherence length
In the focus,
and the wavefront is flat, i.e. . In the case that L^{*}_{1h,v} [cf. (11)] deviates significantly from the geometric distance L_{1}, the focusing becomes intrinsically astigmatic and the horizontal and vertical focus do no longer coincide at a common position L_{2} along the optical axis.
In the focus, the full width at halfmaximum (FWHM) lateral beam size b_{h,v} is minimal,
and has two contributions:
(i) The first contribution is the size of the Airy disc,
described by Abbe's formula (Lengeler et al., 1999). Here, NA_{h,v} is the numerical aperture. The effective aperture D_{h,v} defined in (20) depends not only on the Gaussian aperture function (15) of the optic but is also affected by the Gaussian beam illuminating the optic. As long as the aperture of the optic is illuminated homogeneously, i.e. , the effective aperture is determined by the attenuation in the lens material only. If, however, the beam size is comparable with the effective aperture D_{eff} of the optic, the illumination of the aperture also influences the diffraction limit. In the other extreme case, i.e. for large aperture optics with , the diffraction limit is solely determined by .
(ii) The second contribution is the effective geometric beam size,
that is the image of an effective source with FWHM extension g_{effh,v} demagnified by the factor L_{2h,v}/L^{*}_{1h,v}. In the case of a perfectly incoherent source, b_{effh,v} is the geometric image of the source.
In the focal plane, the FWHM lateral coherence length reduces to
In units of the diffraction limit d_{th,v}, the beam size and the lateral coherence length have the form
and
respectively. They depend only on the ratio of D_{h,v}/2l_{ch,v} or equivalently d_{th,v}/b_{effh,v}. Fig. 3 shows this generic dependence of b_{h,v} and l_{h,v} on the effective image size of the source.
The Airydisc size d_{th,v} depends mainly on the effective aperture D_{eff} [equation (16)] and on the beam size relative to the effective aperture,
Here, d_{t0} is the diffraction limit for homogeneous illumination of the aperture (Lengeler et al., 1999). Fig. 4 shows this dependence expressed in (27). A significant increase of d_{th,v} only occurs when the beam size is significantly smaller than the aperture D_{eff} of the optic. In the more common case, where the aperture is fully illuminated, the diffraction limit is nearly independent of the illumination.
The efficiency of a focusing optic is usually defined by the ratio of the transmitted total F_{0} before and F_{T} after the optic that can, again, each be separated into a horizontal and vertical contribution due to the symmetry of the Gaussian model. The horizontal contribution is
and that incident on the aperture of the optic. Here, we want to analyze what fraction of the undulator radiation can be focused by the optic. For this purpose, we consider the ratio of theAnalogous expressions are found for the vertical contribution. The transmission T separates into a product of two onedimensional transmission functions, T = T_{h} T_{v}, with
where T_{0} is given in equation (15). Just like the Airydisc size, these two quantities depend on the ratio of and D_{eff} only. Fig. 4 shows the dependence of T_{h,v} [given in (28)] on the illuminating beam size . To simplify the presentation, we set the constant T_{0} = 1 in Fig. 4 and in the rest of the article. This corresponds to the case in which the refractive lenses have a negligible thickness d on the optical axis.
in the focus determines the quality of the nanoprobe. From (18)and a similar expression for . The maximal intensity in the focal plane is thus given by
I_{L2} is maximized by maximizing
for both h and v. For given effective aperture D_{eff} and emittance there is an optimal source size. For given source parameters, the optimum is reached for , i.e. for an optic that can capture the full beam.
2.5. Diffractionlimited focusing
As the effective geometric image size b_{effh,v} is made smaller and smaller, the beam size b_{h,v} [cf. equation (22)] is eventually dominated by the size of the Airy disc d_{th,v}. This can be expressed in the form
and serves here as a definition for diffractionlimited focusing. In this case, the transmission is
where is the maximal fraction of the beam that can be focused at the diffraction limit.
In Fig. 3, diffractionlimited focusing is achieved in the gray shaded region. The smaller the effective image b_{effh,v} of the source, the higher becomes the degree of lateral coherence. This is important for coherent Xray diffraction imaging. In these techniques, the sample is illuminated with coherent Xrays and a farfield diffraction pattern is recorded. There are several techniques, amongst which scanning coherent diffraction microscopy, also called ptychography, is one of the most successful (Thibault et al., 2008; Schropp et al., 2011, 2012; Dierolf et al., 2010; Giewekemeyer et al., 2010, 2011; Wilke et al., 2012; Holler et al., 2014).
The statistics of a signal in the diffraction pattern that comes from a certain feature in the sample depend on the fluence on this feature during the exposure of the diffraction pattern (Schropp & Schroer, 2010). This leads to a tradeoff between maximizing intensity and lateral coherence. While there are algorithms that can cope with reduced coherence (Thibault & Menzel, 2013), so far the best results have been obtained with highly coherent beams, i.e. when the lateral coherence length is much larger than the focus size (Schropp et al., 2010).
It is thus useful to introduce a more general criterion for diffractionlimited focusing, requiring
where determines the degree of coherence. The condition = 1 corresponds to the diffractionlimited focusing introduced in (31). For > 1, the coherence in the focus is increased, reducing the transmission through the optic,
accordingly. For an increase in coherence length by and in the horizontal and vertical direction, respectively, the transmission is reduced by .
3. Influence of emittance and source size on the properties of the nanobeam
In the following the influence of the source on the nanobeam properties is discussed. The source properties are significantly different for the horizontal and vertical direction and are, therefore, treated separately. In the Gaussian model for a synchrotron radiation source presented in §2.1, the source is parameterized by the emittance and the source size . The diffraction limit of the source is determined by [cf. equation (1)].
The quantitive results in the following are calculated for a 6 GeV storage ring and a photon energy of E = 12.4 keV (wavelength λ = 1 Å). For this energy a spectroscopy undulator source at PETRA III has the diffractionlimited divergence of = 7.0 µrad on the third harmonic [calculated using equation (1) with parameters from Barthelmess et al. (2008)].
3.1. Horizontal focusing
For nanofocusing, the beam size and lateral coherence length l_{ch} at the optic are the crucial parameters, compared with the effective aperture D_{eff}. Fig. 5 shows the beam size given by (12) as a function of source size for four representative horizontal emittances. The 3.9 and 1 nm rad are horizontal emittances realised by ESRF and PETRA III, respectively. 160 pm rad is the target value for the horizontal emittance for the ESRF within the upgrade proposal for Phase II (Sette, 2012). The 10 pm rad corresponds to a nearly diffractionlimited source at a wavelength of λ = 1 Å (E = 12.4 keV).
The lateral coherence
is largely dominated by the first term, as the lateral coherence length l_{0h} in the source is small, typically only a few hundred nanometers in size for hard Xrays. Its contribution is only relevant near the diffraction limit, when l_{0h}≃ [second term in (34)], or for very large source sizes, when the third term in (34) becomes comparable with the first one. Fig. 5 shows l_{ch} given in (34) for the four different emittances. The lateral coherence length is in most cases much smaller than the lateral beam size, except for the diffractionlimited case ( = 10 pm rad), where the coherence length reaches the beam size for small .
The fraction of the beam that can be focused to the diffraction limit is always smaller than T_{maxh} = as given in (32). It is depicted in Fig. 6. The dependence of T_{maxh} as a function of is relatively flat for the current sources and, therefore, efficient nanofocusing can be realised over a large range of beam sizes. The fraction of the beam that can be focused to the diffraction limit is nearly independent of the β function.
For sources with a smaller emittance, however, the optimum for the focused fraction T_{maxh} as a function of source size becomes more and more pronounced. In the 160 pm rad case, the optimal source size lies at = 5.1 µm and would result in an improvement in efficiency by a factor of 6.1 compared with the PETRA III lowβ case. In the diffractionlimited case ( = 10 pm rad), optimal focusing would be reached for a source size of = 2.75 µm with T_{maxh} = 0.49. The focusing would be about a factor 64 times more efficient in the horizontal direction.
3.2. Vertical focusing
Currently, modern synchrotron radiation sources are not far from being diffractionlimited in the vertical direction at 12.4 keV. Fig. 7 shows the lateral beam size and coherence length l_{cv} given by equations (12) and (13), respectively, as a function of source size for the vertical emittances 10 pm rad (PETRA III), 5 pm rad (minimal coupling at ESRF) and 3.2 pm rad (ESRF Upgrade II), respectively. For the 5 pm rad and 3.2 pm rad cases the lateral coherence length exceeds the beam size for certain source sizes . This illustrates the high degree of lateral coherence in the vertical direction.
Fig. 8 shows the maximal transmitted fraction T_{maxv} of the undulator beam [given by (32)] that can be focused to the diffraction limit. The dots and squares indicate the PETRA III and ESRF vertical source sizes in high and lowβ sections. In terms of optimal use of the beam, the currently given and targeted source sizes are slightly too large, not taking full advantage of the full coherence in the beam. As the lateral coherence l_{cv} can exceed the beam size, large aperture optics that do not cut into the beam can be used in this case. Nearly the full beam can be focused to the diffraction limit in the vertical direction.
The full transmission is calculated as the product T = T_{h}T_{v}. Table 2 summarizes the maximal fraction of the beam that can be focused to the diffraction limit for different existing and potential future synchrotron radiation sources.

4. Conclusion
Today, diffractionlimited focusing is very inefficient. Due to the relatively large horizontal emittance of modern synchrotron radiation sources, only a few photons in a thousand that are emitted from the undulator can at best be transferred into the nanofocus. Future lowemittance storage rings can significantly increase the focusing efficiency. In the diffraction limit, nearly the whole central cone of the undulator could be efficiently focused to the diffraction limit, increasing the focusing efficiency by almost three orders of magnitude.
When the lateral coherence length l_{ch,v} exceeds the beam size by a factor of two, i.e.
the full beam can be focused to the diffraction limit by a largeaperture optic, for which [cf. equation (31)]. According to Fig. 7, this condition can be fulfilled for sufficiently small emittances (in our numerical example for ≃ 5 pm rad or smaller) and an optimized source size. An example of such a large aperture optic could be a large Kirkpatrick–Baez multilayer mirror system (Mimura et al., 2010) that barely truncates the Gaussian beam. For this optic, the diffractionlimiting aperture is defined by the Gaussian beam profile at the optic and
Inserting (35) into (23), the diffractionlimited beam size is
the ultimate intensity is independent of the aperture and given by
With T_{max} = T_{maxh}T_{maxv} ≃ 1, it merely depends on L_{2} and thus on the focal length f of the optic.
For a numerical aperture of NA = 1 mrad and a F_{0} = 10^{13} photons s^{−1}, a maximal intensity of I_{L2} = 6.3 × 10^{9} photons s^{−1} nm^{−2} in a FWHM spot of 53 nm × 53 nm could be reached, exceeding current coherent nanoprobe intensities by at least three orders of magnitude.
ofThe increase in
in the nanobeam would allow for fast scanning and higher signaltonoise ratios, enabling fast imaging of dynamical processes with various Xray analytical contrasts. For coherent Xray diffraction imaging and ptychography, the sensitivity and spatial resolution could be improved to resolve features inside an object that are down to below 1 nm in size. These significant improvements for nanofocusing require an enormous effort to realise a truly diffractionlimited storage ring source. In addition, significant advances are also needed in the field of beamline optics and their stability. Important steps towards this ultimate goal are the construction of the new synchrotron radiation sources MAX IV in Lund, Sweden, and NSLSII at Brookhaven National Laboratory, USA, and the future upgrades of the European Synchrotron Radiation Facility in Grenoble, France, and of the Advanced Photon Source at Argonne National Laboratory near Chicago, USA. With its large circumference of about 2.3 km, PETRA III at DESY in Hamburg, Germany, is well suited for a potential upgrade into a diffractionlimited storage ring.Acknowledgements
The authors thank M. Tischer, DESY, for the discussion on the modeling of undulator radiation. This work is supported by the German Ministry of Education and Research (BMBF) under grant No. 05K13OD4 and by VHVI403 of the Impuls und Vernetzungsfonds (IVF) of the Helmholtz Association of German Research Centres.
References
Barthelmess, M., Englisch, U., Pflüger, J., Schöps, A., Skupin, J. & Tischer, M. (2008). Proceedings of EPAC08. WEPC133. Google Scholar
Born, M. & Wolf, E. (1999). Principles of Optics. Cambridge University Press. Google Scholar
Chu, Y. S. et al. (2008). Appl. Phys. Lett. 92, 103119. Web of Science CrossRef Google Scholar
Dierolf, M., Menzel, A., Thibault, P., Schneider, P., Kewish, C. M., Wepf, R., Bunk, O. & Pfeiffer, F. (2010). Nature (London), 467, 436–440. Web of Science CrossRef CAS PubMed Google Scholar
Giewekemeyer, K., Beckers, M., Gorniak, T., Grunze, M., Salditt, T. & Rosenhahn, A. (2011). Opt. Express, 19, 1037–1050. Web of Science CrossRef CAS PubMed Google Scholar
Giewekemeyer, K., Thibault, P., Kalbfleisch, S., Beerlink, A., Kewish, C. M., Dierolf, M., Pfeiffer, F. & Salditt, T. (2010). Proc. Natl Acad. Sci. USA, 107, 529–534. Web of Science CrossRef CAS PubMed Google Scholar
Holler, M., Diaz, A., GuizarSicairos, M., Karvinen, P., Färm, E., Härkönen, E., Ritala, M., Menzel, A., Raabe, J. & Bunk, O. (2014). Sci. Rep. 4, 3857. Web of Science CrossRef PubMed Google Scholar
Jarre, A., Fuhse, C., Ollinger, C., Seeger, J., Tucoulou, R. & Salditt, T. (2005). Phys. Rev. Lett. 94, 074801. Web of Science CrossRef PubMed Google Scholar
Kang, H. C., Yan, H., Winarski, R. P., Holt, M. V., Maser, J., Liu, C., Conley, R., Vogt, S., Macrander, A. T. & Stephenson, G. B. (2008). Appl. Phys. Lett. 92, 221114. Web of Science CrossRef Google Scholar
Kohn, V. G. (2003). J. Exp. Theoret. Phys. 97, 204–215. Web of Science CrossRef CAS Google Scholar
Lengeler, B., Schroer, C., Tümmler, J., Benner, B., Richwin, M., Snigirev, A., Snigireva, I. & Drakopoulos, M. (1999). J. Synchrotron Rad. 6, 1153–1167. Web of Science CrossRef IUCr Journals Google Scholar
Mimura, H., Handa, S., Kimura, T., Yumoto, H., Yamakawa, D., Yokoyama, H., Matsuyama, S., Inagaki, K., Yamamura, K., Sano, Y., Tamasaku, K., Nishino, Y., Yabashi, M., Ishikawa, T. & Yamauchi, K. (2010). Nat. Phys. 6, 122–125. Web of Science CrossRef CAS Google Scholar
Mimura, H., Yumoto, H., Matsuyama, S., Sano, Y., Yamamura, K., Mori, Y., Yabashi, M., Nishino, Y., Tamasaku, K., Ishikawa, T. & Yamauchi, K. (2007). Appl. Phys. Lett. 90, 051903. Web of Science CrossRef Google Scholar
Schroer, C. G., Boye, P., Feldkamp, J. M., Patommel, J., Samberg, D., Schropp, A., Schwab, A., Stephan, S., Falkenberg, G., Wellenreuther, G. & Reimers, N. (2010). Nucl. Instrum. Methods Phys. Res. A, 616, 93–97. Web of Science CrossRef CAS Google Scholar
Schroer, C. G., Brack, F.E., Brendler, R., Hönig, S., Hoppe, R., Patommel, J., Ritter, S., Scholz, M., Schropp, A., Seiboth, F., Nilsson, D., Rahomäki, J., Uhlén, F., Vogt, U., Reinhardt, J. & Falkenberg, G. (2013). Proc. SPIE, 8848, 884807. CrossRef Google Scholar
Schroer, C. G., Kurapova, O., Patommel, J., Boye, P., Feldkamp, J., Lengeler, B., Burghammer, M., Riekel, C., Vincze, L., van der Hart, A. & Küchler, M. (2005). Appl. Phys. Lett. 87, 124103. Web of Science CrossRef Google Scholar
Schroer, C. G., Schropp, A., Boye, P., Hoppe, R., Patommel, J., Hönig, S., Samberg, D., Stephan, S., Schöder, S., Burghammer, M., Wellenreuther, G. & Falkenberg, G. (2011). AIP Conf. Proc. 1365, 227–230. CrossRef Google Scholar
Schropp, A., Boye, P., Feldkamp, J. M., Hoppe, R., Patommel, J., Samberg, D., Stephan, S., Giewekemeyer, K., Wilke, R. N., Salditt, T., Gulden, J., Mancuso, A. P., Vartanyants, I. A., Weckert, E., Schöder, S., Burghammer, M. & Schroer, C. G. (2010). Appl. Phys. Lett. 96, 091102. Web of Science CrossRef Google Scholar
Schropp, A., Boye, P., Goldschmidt, A., Hönig, S., Hoppe, R., Patommel, J., Rakete, C., Samberg, D., Stephan, S., Schöder, S., Burghammer, M. & Schroer, C. G. (2011). J. Microsc. 241, 9–12. Web of Science CrossRef CAS PubMed Google Scholar
Schropp, A., Hoppe, R., Patommel, J., Samberg, D., Seiboth, F., Stephan, S., Wellenreuther, G., Falkenberg, G. & Schroer, C. G. (2012). Appl. Phys. Lett. 100, 253112. Web of Science CrossRef Google Scholar
Schropp, A. & Schroer, C. G. (2010). New J. Phys. 12, 035016. Web of Science CrossRef Google Scholar
Sette, F. (2012). ESRF Upgrade Programme Phase II. Technical Report. ESRF, Grenoble, France. Google Scholar
Singer, A. & Vartanyants, I. A. (2014). J. Synchrotron Rad. 21, 5–15. Web of Science CrossRef IUCr Journals Google Scholar
Thibault, P., Dierolf, M., Menzel, A., Bunk, O., David, C. & Pfeiffer, F. (2008). Science, 321, 379–382. Web of Science CrossRef PubMed CAS Google Scholar
Thibault, P. & Menzel, A. (2013). Nature (London), 494, 68–71. Web of Science CrossRef CAS PubMed Google Scholar
Thompson, A. C., Attwood, D., Gullikson, E., Howells, M. R., Kim, K.J., Kirz, J., Kortright, J. B., Lindau, I., Liu, Y., Pianetta, P., Robinson, A., Scofield, J. H., Underwood, J. H., Williams, G. P. & Winick, H. (2009). Xray Data Booklet. Lawrence Berkeley National Laboratory, Berkeley, CA, USA. Google Scholar
Vartanyants, I. A. & Singer, A. (2010). New J. Phys. 12, 035004. Web of Science CrossRef Google Scholar
VilaComamala, J., Diaz, A., GuizarSicairos, M., Mantion, A., Kewish, C. M., Menzel, A., Bunk, O. & David, C. (2011). Opt. Express, 19, 21333–21344. Web of Science PubMed Google Scholar
Vogt, S. & Lanzirotti, A. (2013). Synchrotron Radiat. News, 26(2), 32–38. CrossRef Google Scholar
Wilke, R. N., Priebe, M., Bartels, M., Giewekemeyer, K., Diaz, A., Karvinen, P. & Salditt, T. (2012). Opt. Express, 20, 19232–19254. Web of Science CrossRef CAS PubMed Google Scholar
Xu, H., Wu, Z. & Tai, R. (2013). J. Phys. Conf. Ser. 463, 011001. CrossRef Google Scholar
Yan, H., Rose, V., Shu, D., Lima, E., Kang, H. C., Conley, R., Liu, C., Jahedi, N.,Macrander, A. T., Stephenson, G. B., Holt, M., Chu, Y. S., Lu, M. & Maser, J. (2011). Opt. Express, 19, 15069–15076. Web of Science CrossRef CAS PubMed Google Scholar
This is an openaccess article distributed under the terms of the Creative Commons Attribution (CCBY) Licence, which permits unrestricted use, distribution, and reproduction in any medium, provided the original authors and source are cited.