Table-top laser-based proton acceleration in nanostructured targets

PAPER • OPEN ACCESS Table-top laser-based proton acceleration in nanostructured targets To cite this article: M Blanco et al 2017 New J. Phys. 19 033004 View the article online for updates and enhancements. Related content Review of laser-driven ion sources and their applications Hiroyuki Daido, Mamiko Nishiuchi and Alexander S Pirozhkov - Short pulse laser interaction with microstructured targets: simulations of laser absorption and ion acceleration O Klimo, J Psikal, J Limpouch et al. - Enhanced ion acceleration in transition from opaque to transparent plasmas R Mishra, F Fiuza and S Glenzer - Recent citations Enhancement of laser-driven ion acceleration in non-periodic nanostructured targets J. Ferri et al - Generation of ultra-energetic ions by interaction of petawatt lasers with micrometer-scale foils A. Héron et al - Target normal sheath ion acceleration by fs laser irradiating metal/reduced graphene oxide targets L. Torrisi et al - This content was downloaded from IP address 83.36.121.176 on 04/06/2020 at 11:23 New J. Phys. 19 (2017)033004 https://doi.org/10.1088/1367-2630/aa5f7e PAPER Table-top laser-based proton acceleration in nanostructured targets M Blanco 1 , M T Flores-Arias 1 , C Ruiz 2 and M Vranic 3 1 Photonics4Life Research Group, Departamento de Física Aplicada, Facultade de Física, Universidade de Santiago de Compostela, Campus Vida s/n,15782 Santiago de Compostela, Spain 2 Instituto Universitario de Física Fundamental y Matemáticas and Departamento de Didáctica de la Matemática y de las Ciencias Experimentales, Universidad de Salamanca, Patio de las Escuelas s/n, Salamanca, Spain 3 GoLP/Instituto de Plasmas e Fusão Nuclear, Instituto Superior Técnico, Universidade de Lisboa, 1049-001 Lisbon, Portugal E-mail: [email protected] and maite.fl[email protected] Keywords: laser-plasma interaction, particle in cell simulations, laser-driven acceleration, nanostructured targets, laser ion acceleration, TNSA Abstract The interaction of ultrashort, high intensity laser pulses with thin foil targets leads to ion acceleration on the target rear surface. To make this ion source useful for applications, it is important to optimize the transfer of energy from the laser into the accelerated ions. One of the most promising ways to achieve this consists in engineering the target front by introducing periodic nanostructures. In this paper, the effect of these structures on ion acceleration is studied analytically and with multidimensional particle-in-cell simulations. We assessed the role of the structure shape, size, and the angle of laser incidence for obtaining the efficient energy transfer. Local control of electron trajectories is exploited to maximize the energy delivered into the target. Based on our numerical simulations, we propose a precise range of parameters for fabrication of nanostructured targets, which can increase the energy of the accelerated ions without requiring a higher laser intensity. 1. Introduction Ion acceleration in laser-driven plasma accelerators has been a very active field in the last few years. It has been demonstrated that it is possible to accelerate ions up to energies of tens of MeV with table top laser sources [1–3]. One of the most robust mechanisms used to accelerate ions in plasma based accelerators is the target normal sheath acceleration (TNSA). In this mechanism a high intensity laser interacts with a few-micron thick solid target to produce energetic ions [4–7]. The laser pulse ionizes the target surface and heats up the electrons; these electrons propagate across the target and escape perpendicularly to the rear surface. This generates a space charge separation in the rear surface that yields a strong longitudinal field which can accelerate positively charged particles located in the vicinity of the surface. Solid targets for plasma-based accelerators can be manufactured with a variety of properties to make the acceleration more efficient. This subject has received a wide attention because the optimization of the targets opens a way to produce more energetic ions without the need of increasing the laser power. Different approaches such as varying the target thickness [8], nanostructuring the back surface of the target [9,10]or growing a layer of low density foam [11–13]have already been studied. Several publications have reported that adding periodic nanostructures on the target front surface enhances drastically the laser energy absorption [13–21]. This generates ions with much higher energies than the ones obtained when targets with a flat surface are used [13,20–30]. The nature of this enhancement is still a matter of discussion, however it is known that it is strongly dependent on the shape of the structures, as well as on the angle of incidence of the impinging laser [13– 15,17,18,21,22,26,27]. As there are several laser absorption mechanisms in overdense plasmas, such as the generation of surface plasma waves (SPW)[13,15,16,29,31–35], resonant absorption, vacuum heating or J×Bheating [36–38], one can use nanostructures with properties especially suited to enhance a particular absorption mechanism. Our aim OPEN ACCESS RECEIVED 30 November 2016 REVISED 19 January 2017 ACCEPTED FOR PUBLICATION 9 February 2017 PUBLISHED 1 March 2017 Original content from this work may be used under the terms of the Creative Commons Attribution 3.0 licence. Any further distribution of this work must maintain attribution to the author(s)and the title of the work, journal citation and DOI. © 2017 IOP Publishing Ltd and Deutsche Physikalische Gesellschaft is to optimize the acceleration of electrons in the vacuum gaps of a periodic structure, so-called vacuum heating [17,21,27]. The main purpose of this work is to show how the geometry of periodic structures can be optimized to achieve a higher laser energy absorption and proton energies, in particular for the specification of the STELA laser of the L2A2 facility of the University of Santiago de Compostela, with laser intensities on the order of 1 019 Wcm −2 and a peak power on the order of tens of TW. We present an analytical and numerical study of the interaction of laser pulses and solid targets with triangular periodic nanostructured surfaces. The dimensions of the structures dictate the time electrons spend interacting with the laser field in the free spaces within the structure which directly influences the ratio of laser energy absorbed by the electrons. The reason behind the observed enhanced absorption and higher proton energies is the possibility to control the recollision time of the electrons by changing the parameters of the triangular structure. We propose an optimal structured surface for energy absorption and energetic proton production that can be fabricated and used experimentally, providing a robust strategy to obtain higher energy protons without the need of using a higher laser intensity. We introduce a simple analytical model for the laser energy absorption by the plasma electrons as a function of the nanostructure dimensions. The predictions of this model are in good agreement with our particle-in-cell (PIC)simulation results. In addition, we study the effects of using oblique laser incidence, and propose an alternative structured target surface optimized for oblique incidence. This paper is structured as follows: section 2introduces an analytical model to account for the increase in the energy absorption due to the presence of the periodic nanostructures. Section 3contains 2D PIC simulations, where a wide range of parameters was studied to find the optimal target design for maximal laser absorption and proton cutoff energy. Section 4accounts for differences between 2D and 3D geometry. The effect of using oblique incident laser pulses is adressed in section 5, in which we propose an optimal experimental configuration to obtain energetic protons. The summary and discussion of our results are presented in sections 6 and 7. 2. Analytical model of electron dynamics In this section we introduce a simple analytical model to understand the electron motion in the presence of the laser field within the periodic structures. The laser energy absorption is directly related to the electron heating, as electrons are the lightest particles in the plasma and the first to interact with the laser field. Understanding how electrons absorb the laser energy and carry it towards the rear of the target is crucial to select an optimal surface structure. The use of triangular structures in the front face of the target changes the local angle of incidence of the laser and allows electrons to undergo a temporary interaction with the laser field in vacuum before recolliding with the target. As the laser arrives to the target, it strips off a portion of the electrons from the lateral surface of the structure. The electrons are accelerated by the laser field in the vacuum gaps of the structures and gain energy. They reenter the target where the laser cannot penetrate and deliver their energy into the target, as shown in figure 1. The shape of the triangular structures determines the time the electrons spend being accelerated in the vacuum gap and their recollision energy. We expect an optimal laser absorption for targets withgeometrical properties that allow for maximum electron energy gain. A simple model that neglects all fields except the laser is useful to understand how the recollision energy is related to the triangle shape. Our starting point is to consider the relativistic motion of an electron in vacuum under the influence of a linearly polarized electromagnetic wave given by the vector potential j=w  ()ˆ A axsin mc 0 2 e, where a 0 is the dimensionless vector potential defined by = l m - () a 0.85 I 010 W cm m 2 18 2 2 1 2, where Iis the laser intensity in W cm-2and λthe laser wavelength in μm. The variable j wj=- +  ·tkr 0 represents the electromagnetic wave phase,  k is the wave vector,  r the particle position, ωthe angular frequency, tthe time and j 0is the initial phase. The equation of motion of an electron in the vacuum gap is determined by the Lorentz force: gg =- - ´ = ¶ ¶-´´  ⎛ ⎝ ⎜⎞ ⎠ ⎟⎛ ⎝ ⎜⎞ ⎠ ⎟ () () p tqE q p mc Bq c A tqp mc A d d,1 ee e e where q e is the electron charge. This equation can be solved for the specified vector potential assuming that the electron is initially at rest and that for t=0 we have j =0. The momentum and displacement of the electron are then given by [36]: jj==() () ()pamc p amc 2sin sin , 2 1 0 2 e2 20e 2 New J. Phys. 19 (2017)033004 M Blanco et al plj j plj D= - D= ⎜⎟ ⎜⎟ ⎛ ⎝ ⎞ ⎠ ⎛ ⎝ ⎞ ⎠ () ()xaxa 8 sin 2 2sin 2,3 10 2 2 02 where the indexes ‘1’and ‘2’refer to the longitudinal and transverse field directions and l p w =c2is the laser field wavelength. The maximum electron energy is reached when j p=2, because both components of the electron momentum are maximized, so if the electrons reenter the target at this point they will absorb the maximum possible energy from the field. Reaching the optimal phase at the moment when the electron reenters the target is controlled by its initial position in the structured surface, expressed by its initial height, h 0 . We can establish a relation between the initial height where a single electron is located and the phase when it arrives to the surface of the next triangle by using the displacements in equation (3). This relation is obtained from the following relation for the triangle angle: a===-() () h w x x h x tan 2,4 f fo 1 2 0 2 where hand ware the structure height and width and the indexes ‘o’and ‘f’indicate original and final position at the periodic structure surface, respectively. Taking into account the definition of the displacements D º-∣ ∣ xxx fo , we can obtain the final equation =D +Dhx x h w 01 1 22 , which, written in our variables of interest, is: jplj j plj =- + ⎜⎟ ⎜⎟ ⎛ ⎝ ⎞ ⎠ ⎛ ⎝ ⎞ ⎠ () () ()haah w16 sin 2 2sin 2.5 00 202 The maximum amount of energy absorbed by the electrons in the gap is reached when jp=»()hh2 0 , because this means that the electrons initially located at the tip of the structure gain the maximum possible energy. These electrons are the first to interact with the laser pulse. If jp=>()hh2 0 the electrons will not reach the maximum energy because their ideal initial height is not allowed on the structure and when jp=<()hh2 0 a portion of the electrons at the top of the structure will stay longer in the vacuum gaps and not enter the target with the optimal energy. It can be also noted that the second term on the right hand side of equation (5)becomes less relevant as a 0 increases. However, the findings of equation (5)cannot be applied directly to very high intensities where the hole-boring can destroy the pre-formed structures before the end of the interaction. We therefore restrict our analysis to a moderate laser intensity. Using a laser field with a dimensionless amplitude of = a 4 0 , which can be achieved with the laser STELA, the equation (5)for the maximum electron energy becomes: Figure 1. Illustration of the electron dynamics over a laser period T, taken from a PIC simulation, with six snapshots of the electron density, the E 2 component of the electric field, in which the laser field is polarized, and the most energetic electrons, colored depending on their kinetic energy. The electrons move in the vacuum gap from one triangle to the next according the sign of the E 2 component of the electromagnetic field, gaining energy in the process. 3 New J. Phys. 19 (2017)033004 M Blanco et al jp l p l ==+() ()hwh22 2.6 0 The value of h 0 relative to hin the previous equation is controlled by the width of the structures. For lp w 2then h h 0and viceversa. Therefore, there is an optimal structure width for improving the energy absorption, given by l= w 0.64 . When the structure width has this value, equation (6)becomes jp l==+()hh22 0, which means that for higher structures l ( )h2we get h h 0. We therefore expect that above a certain structure height l~ ( )h0.5 the energy absorption percentage reaches a maximum value and does not change further. This simple model provides a clear picture on how the engineering of the triangular structures can be used to control the electron trajectories and maximize the energy they deliver to the target. Figure 2depicts the energy and motion of an electron under equations (2)and (3)and shows that the structure shape can be manipulated to obtain maximum absorption from the electrons moving from the tip of one triangle across the vacuum gap. Figure 2(a)shows that there is a maximum energy, reached periodically for certain positions that would correspond to the phase j p=+()N212 , where Nis an integer. Figures 2(b)and (c)show, for different structure heights and widths, the trajectory of an electron moving in the vacuum gap, colored according to its energy. It can be observed that the shape of the structure influences the energy that the electron has at the recollision time; the energy is lower in figure 2(b)than in 2(c). The predictions obtained from the model for the dependence of the energy absorption with the structure height and width can be tested by performing PIC simulations. In the following sections we discuss the results obtained from such simulations, with the aim of designing an optimal target for energy absorption and ion acceleration. 3. Effect of the structure shape and size on the laser energy absorption and proton acceleration The aim of this section is to identify a parameter range with maximum transfer of laser energy to the accelerated protons. To adress how the shape of the structures affects the absorption of laser energy as well as the energies of the electrons and protons, we present a numerical study encompassing a wide range of sizes for two types of structures indicated in figure 3. We vary their width and height and use a laser pulse at normal incidence. Numerical simulations of the laser-plasma interaction are performed with the PIC code OSIRIS [39].In OSIRIS, the fields are stored on a discretized spatial grid and advanced according to the Maxwell’s equations. The particle motion is determined by the relativistic Lorentz force. Two different targets with triangular structures were used in this work, as shown in figure 3. The reasons behind choosing these structures are that they yield high absorption rates and efficient proton acceleration in comparison with other kinds of structures [18,22]and can be manufactured for their use in experiments. The asymmetry presented in figure 3(c)(‘tilted triangles’)with respect to figure 3(b)(‘regular triangles’)is interesting from the experimental point of view, where oblique incident laser pulses are going to be used. The targets are made of electrons and protons with a number density of = n n40 c , where = w p n m q c4 e2 e 2 is the critical plasma density. All the targets have a bulk thickness of l 0 .5 (unless specified differently), where λis the wavelength of the laser, and the number of particles per cell is 16 per species. The density has a steep profile as we Figure 2. (a)Energy of one electron versus the longitudinal coordinate x 1 and its trajectory. The trajectory is colored according to its energy. Electron trajectories within the vacuum gaps colored according to their energy for different structure heights and widths: (b) l=h0.5 and l= w 0.25 , and (c)l=hand l= w 0.7 . The dotted line represents the surface where the electron reenters the target. All panels are for a dimensionless vector potential of = a 4 0. 4 New J. Phys. 19 (2017)033004 M Blanco et al consider a high contrast laser > ( 10 10 at 5 ps)which corresponds to the STELA laser. The simulation box has a width and length of m 3 8.3 m and 16.9 μm, respectively. The spatial resolution is d =2.55 nm in both axes. The laser pulse is focused on the target surface. This pulse is launched from the left wall of the simulation box, located at a distance of m8.9 m to the target. The laser has an intensity of ´ 3 .45 10 19 Wcm −2 , a FWHM of 25 fs (with a sin 2 temporal profile), a wavelength of l =800 nm and a spot diameter of m6m . The laser pulse is linearly polarized in the simulation plane, such that it is always p-polarized in relation to the structures. The simulation advances in timesteps of 4.26 as. The reflected energy, as well as the electron properties at the rear surface, are measured right after the interaction finishes, at the time 70.2 fs. The proton properties are measured at 172.3 fs, the time at which electrons that generate the accelerating field start leaving the simulation box. The reflected energy is measured by integrating the reflected field energy density. We have also monitored the electron and proton kinetic energy, as well as the energy of the self-consistent fields generated around the target. The energy conservation has been verified throughout all the simulations. The electron temperature at the rear surface is obtained by fitting the electron spectrum to a Maxwell–Jüttner distribution. The simulation setup is designed to scan the parameter space and compare the relative gain between the flat and structured targets. Several cases from low to almost complete laser absorption are illustrated in figure 4,figure 4(a)shows the incident laser pulse and figures 4(b)–(e)display the reflected fields. The lowest absorption is obtained for a flat target. The results obtained for different structured targets are displayed in figures 4(c)–(e). We observe that the reflected spatial distribution of light when structured targets are used carries the imprint of the nanostructures at the target surface, and more laser energy is absorbed. Figure 3. Shapes of the triangular structures. (a)3D image of the simulation setup and (b),(c)detailed view of the 2D targets. The variable hrepresents structure height, wthe width, θthe angle formed between two neighboring structures and αthe angle of lase incidence towards the target. Figure 4. (a)Incident and (b)–(e)reflected electromagnetic energy density for different structured targets. The reflected field is shown for a (b)flat target and targets with structure height and width of: (c)l=hand l= w 0.25 ,(d)l=h0.25 and l= w and (e)l=h and l= w 0.7 . 5 New J. Phys. 19 (2017)033004 M Blanco et al To verify the predictions of section 2, we perform a first set of simulations with a fixed structure height of l=h , where we vary the structure width. According to our analysis we should expect maximum energy absorption at a width of l~ w 0.64 . Figure 5(a)shows the energy absorption, as a function of the structure width, for regular and tilted triangular nanostructures. In both cases the energy absorption increases with the width of the triangles up to a maximum nanostructure width around l 0 .7 . Above this value the energy absorption decreases smoothly as the triangle width increases. For the triangles ll– 0 .6 wide, we obtain that the energy absorption is above 90%. The increase in electron temperature is shown in figure 5(b): it rises with the width of the triangles for both types of structures. Once the width of the triangles becomes close to l 0 .7 the slope of the curve changes to a lower value. The gain in proton cutoff energy is shown in 5(c). It exibits a similar trend as the energy absorption. The plots in figure 5show that the the structure width can be optimized to yield a maximum laser absorption and proton energy cutoff. The structure width of the optimal target is consistent with the analytically predicted l= w 0.64 . A second set of simulations is performed with a fixed structure width of l= w 0.7 and varying the structure height. We kept the rest of simulation parameters equal to the ones in the previous case. Here we should expect nearly a complete laser energy absorption above a certain threshold structure height. Figure 6displays the energy absorption, the relative electron temperature and proton cutoff energy versus the height of the structures. The energy absorption percentage is shown in figure 6(a), that depicts an increase of the absorption of energy as the height of the triangles becomes bigger, up to a maximum value, close to 100%. Once this maximum is achieved, it remains unchanged as we increase the height of the triangles. The electron temperature, in figure 6(b), shows a big increase when the structures are added, followed by a smooth decay/stabilization for higher structures. Figure 6(c)displays the relative proton cutoff energy. For l>h0.5 , the results in figure 6show that the absorption percentage is above 90% and there is a five-fold increase in the proton cutoff energy compared with the flat target. The high absorption percentages shown in figure 6(a)are due to the choice of a structure width of l 0 .7 , close to the optimal value found before. As predicted by the analytical model, above the threshold structure height, the laser energy absorption is nearly 100% and there is no significant difference observed in the spectrum of generated protons. Figure 5. (a)Laser energy absorption percentage, (b)electron temperature and (c)proton cutoff energy as a function of the structure width. The height of the structures is l=h. The electron temperature and proton energy are normalized to the values obtained for a flat target. Figure 6. (a)Laser energy absorption percentage, (b)electron temperature and (c)proton cutoff energy as a function of a structure height. The width of the structures is l= w 0.7 . The electron temperature and proton energy are normalized to the values obtained for a flat target. 6 New J. Phys. 19 (2017)033004 M Blanco et al Figures 5and 6demonstrate that there is a correspondence between the trend followed by the laser absorption and the cutoff energy of the protons. This is not surprising, because in TNSA the absorbed laser energy is carried by the electrons towards the rear side of the target. These electrons escape the target and create a longitudinal field proportional to the square root of the electron temperature and to the electron front number density [6]. This longitudinal field is responsible for the acceleration of protons. We therefore expect higher proton energies for higher achieved electron temperatures at the rear surface. However, additional height in the structures changes the effective target thickness and hence the electron front number density is also modified. The consequence is that the electrons with a lower temperature (e. g. for l=h1.5 in figure 6(b)) can, in principle, generate the accelerating field of the same magnitude as the electrons with a 53% higher temperature in a case with a different effective target thickness (e. g. for l=h0.5 in figure 6(b)). We therefore obtain similar values for the accelerating field and for the proton cutoff energy in all cases where l>h0.5 . 4. Comparison between 2D and 3D results We have analyzed how the energy absorption varies when triangular structures are on the target surface and how this variation affects the electron heating and consequently the energies of the accelerated protons. Our theoretical analysis, combined with 2D PIC simulations, shows that the structure shape can be optimized to yield high percentages of energy absorption, which is in agreement with previous publications [17,21,27]. The values obtained for the optimal height and width in terms of energy absorption are given by a width of = w 512 nm and a lower bound for the structure height of ~h400 nm. Fabrication of these structures is achievable by current techniques, therefore the targets described here can be manufactured in a cost effective way and used experimentally [13,18,22,23]. Our conclusions regarding the target structure for optimal laser absorption are general and can be extended to 3D geometry. The electron interaction with an electromagnetic wave in vacuum is fully described in 2D. The energy of the electrons at the point of re-entry into the target depends on the geometrical properties of the structures such as width and height and it is intrinsically a 2D problem. The optimal configuration for laser absorption is therefore likely to be the same in 2D and 3D geometry. However, even though ion acceleration can be studied qualitatively in 2D, it is well-known that the proton energy cutoff in TNSA is lower in 3D geometry [40,41]. Due to limited computational resources, it is not possible to perform a full-scale 3D simulation and allow enough time for target expansion. However, the 3D simulations can be performed in slab geometry. In this geometry the laser is treated as a wavepacket that is transversely a plane wave and periodic transverse boundary conditions are applied both for the fields and the particles, except for the direction of laser propagation where open boundaries are used. The simulation box is l25 long and ll´ 3 .5 3.5 wide. The laser pulse is initialized inside the box with a total duration of T 7 , where l=Tcis the laser period, and a distance of l 0 .5 to the structure tip. We performed simulations for optimal structured targets where l=h and l= w 0.7 and for flat targets, with a goal to compare the relative increase of the absorption efficiency in 2D and 3D. In 3D simulations we obtained 91.5% of laser absorption for regular, 89.5% for tilted triangles and 2% for a flat target. In 2D simulations, the 95.4% was absorbed for regular, 92.3% for tilted triangles, and 2.6% for the flat target. The absorption estimates from 2D and 3D are consistent within a margin of 4%. There is approximately a 15-fold increase in the proton cutoff energy when we use structured targets instead of flat ones in 3D. The electron spectra from 2D and 3D simulations at the time 25.5 fs are displayed in figure 7(a). They are normalized to the same reference height at the energy 2 MeV. We can observe a slight difference between the tilted and regular structures, due to different electron dynamics at the target surface. The respective proton spectra at the time 51.1 fs are shown in figure 7(b). These spectra are normalized to the same reference height at the energy 1 MeV. As expected, the proton cutoff is lower in 3D compared to the 2D case. Apart from verifying the conclusions obtained in 2D, an additional advantage of 3D simulations is that they can provide an estimate of the total number of accelerated protons. In our case the number of protons being accelerated to an energy above 0.1 MeV is approximately 1.35×10 11 , corresponding to over ~21.6 nC of charge accelerated to energies up to 4 MeV. As the transverse box dimensions are chosen to be on the order of the laser spotsize, this is the approximate number of protons per shot expected in an experiment with similar conditions. 5. Oblique laser incidence In the previous sections it has been discussed how the energy absorption and the particle properties change with the front structure shape of the solid target. All the previous simulations have been performed with a pulse in normal incidence, however experiments of TNSA proton acceleration are typically done in oblique incidence. 7 New J. Phys. 19 (2017)033004 M Blanco et al The main reason for using oblique incidence is to avoid the damage on the optical elements used to transport the beam to the target, with the particles ejected by the target or the back reflection of the laser pulse. The angle of incidence of the laser pulse is expected to affect the laser energy absorption and the particle energies. We have performed simulations at different angles of incidence using targets with l= w and l=h1.2 , for regular and l= w and l=h for tilted triangles. Figure 8displays (a)the energy absorption, (b)the electron temperature and (c)the proton cutoff energy at oblique laser incidence. Figure 8(a)shows that for the regular triangular structure, the maximum absorption and particle energies occur at normal incidence, while for the tilted structures this maximum is shifted by a value close to 22.5o. The electron temperature for the tilted structures, in 8(b), displays two maxima at the angles 22.5 o , while the proton cutoff energy for the same structure, in 8(c), shows a plateau around the zero angle slightly maximized for the maximum energy absorption angle. The peak observed for the elecron temperature at a=-22.5 o represents electrons that get heated efficiently but do not contribute to enhance the energy of TNSA protons. This behavior suggests that a SPW [16,29,31–35] is being excited at this angle, such that the electrons escape the target tangentially. This is confirmed by measuring the longitudinal accelerating field in the rear surface of the target, which shows the same trend as the proton cutoff energy in figure 8(c). The analysis of the effect of oblique incident pulses shows that the asymmetric tilted triangles yield to a higher absorption percentage and more energetic protons at oblique incidence compared to normal incidence. We have performed an additional simulation combining an oblique incident laser pulse with an optimized height and width of the structure l=h and l= w 0.7 . The bulk target thickness is l2and the angle of incidence of the laser is a=17.5o. The comparison between the results obtained with the same setup for a target with a flat surface and the structured target show a 15-fold increase in the energy absorption percentage, from a 6.1% in the flat target to a 90.6% in the structured target. This enhancement of the energy absorption generates protons with energies between 4 and 5 times higher compared with the case in which a flat solid target was used. This is verified in figure 9that shows (a)the proton energy spectrum and the momentum space –pp 1 2 of the protons. Both, the Figure 7. The spectrum of (a)electrons and (b)protons measured for the 2D and 3D setup. The height and width of the structures are l=hand l= w 0.7 . Figure 8. (a)Laser energy absorption percentage, (b)electron temperature and (c)proton cutoff energy. The gray dotted line indicates the angle of incidence a=22.5 o , where the maximum energy absorption for the tilted structure occurs. The width and height of the structures are l= w and l=hfor the tilted triangular structure and l=h1.2 for the regular triangular structure. The values are normalized to the results obtained for a flat target and a normally incident laser pulse. 8 New J. Phys. 19 (2017)033004 M Blanco et al