Parametric Study of Proton Acceleration from Laser-Thin Foil Interaction

Abstract

We experimentally investigated the accelerated proton beam characteristics such as maximum energy and number by varying the incident laser parameters. For this purpose, we varied the laser energy, focal spot size, polarization, and pulse duration. The proton spectra were recorded using a single-shot Thomson parabola spectrometer equipped with a microchannel plate and a high-resolution charge-coupled device with a wide detection range from a few tens of keV to several MeV. The outcome of the experimental findings is discussed in detail and compared to other theoretical works.

1. Introduction

The acceleration of protons and ions during the interaction of high-power laser pulses with solid targets has been a well-investigated field since the first experimental study in the 1980s [1]. Thanks to the rapid advancement of high-power laser and optical technology, the focused intensities on targets exceed ${10}^{18}\mathrm{W}/{\mathrm{cm}}^2$ and the maximum kinetic energy of the accelerated protons reached tens of megaelectronvolts ($\mathrm{MeV}$) [2]. The acceleration process occurs over a relatively very short length in the order of sub-millimeters and the generated proton beams possess high-emittance, laminarity and a short duration [3,4]. These characteristics of the proton beams generated from the interaction extend their huge potential in a plethora of applications, such as fusion energy [5,6], medical applications [7], isotope production [8] and astrophysical modeling [9,10].

Ion acceleration is the most efficient and is suitable for secondary applications when it is generated from the rear surface of the interacting solid target. Indeed, several models were proposed to describe the emission of the positively charged particles from the rear surface of the irradiated target, such as target normal sheath acceleration (TNSA) [11] and radiation pressure acceleration (RPA) [12], or even both in a hybrid acceleration scheme [13]. A detailed review of all the possible ion acceleration processes during laser–matter interaction can be found in review articles [4,14,15]. For laser intensities $\sim {10}^{19}\mathrm{W}/{\mathrm{cm}}^2$, the TNSA mechanism is the most dominant process; hence, we will focus on the TNSA process in this work. In this model, the fast electrons accelerated by the laser at the irradiated side propagate through and then exit the target, forming a dense sheath at the rear side of the foil. As a result, a huge electrostatic field in the order of $\mathrm{TV}/\mathrm{m}$ is generated due to the charge separation of escaping electrons and the unbalanced charge left behind. This field can ionize and accelerate the atoms at the rear side of the target [11]. The accelerated ions and protons mainly originate from the hydrogen-rich contamination layer and water vapor at the target rear surface. TNSA generally produces broad Maxwellian-like proton and ion energy spectra with an exponentially decreasing profile with increasing ion energy [16], with a sharp cutoff. This was attributed to charge separation, which limits the ion velocities by forming a non-neutral electrostatic sheath, which diminishes the exponential density profile [17].

Since direct ion acceleration can not be yet realized directly by current laser technology, it has to rely on a driving electron component to transfer the energy from the laser to the ions. It has been found that the maximum energy of the accelerated protons is proportional to the temperature of the hot electrons creating the sheath as ${\mathrm{E}}_{\mathrm{proton}}\approx \beta {\mathrm{T}}_{\mathrm{hot}}$ [18]; the beta factor will be defined later for various parameters. Different models were suggested to explain the origin of the energetic electrons from the irradiated front side of the target, for example, collisional heating such as inverse bremsstrahlung, collisionless heating such as resonance absorption [19], vacuum heating [20] and pondermotive acceleration [21] depending on the laser and target parameters. When a high-intensity laser pulse reaches the target surface, the intense part of the pulse will not directly interact with the bulk material of the target, but with a pre-plasma generated by the advancing pedestal of the intensity profile of the laser due to the amplified spontaneous emission (ASE). If a p-polarized laser pulse is incident at an angle $\theta$ at a pre-plasma with a gradient length of ${\lambda }_g$, the laser light will propagate up to the density ${\mathrm{n}}_{\mathrm{cr}}{cos}^2\theta$ before it is specularly reflected; as a result, the electric field vector $\overrightarrow{E}$ of the laser becomes parallel to the density gradient $\overrightarrow{▽}n$. For relatively long ${\lambda }_g$ (sub-wavelength or larger), an electron plasma wave can be resonantly excited along the direction of the density gradient, and part of the laser energy is transferred to the electrons. This is called resonance absorption, [22] and the electron temperature scales as ${\mathrm{T}}_{\mathrm{hot}}\propto {\left(\mathrm{I}{\lambda }^2\right)}^{1/3}$. For sharp density gradients, however, vacuum heating or Brunel absorption [20] becomes important; in this case, a strong energy absorption can be accounted for by the electrons that are dragged into the vacuum and then sent back into the plasma with velocities equivalent to the quiver velocity ${\mathrm{v}}_{\mathrm{osc}}=\mathrm{eE}/{\mathrm{m}}_{\mathrm{e}}\omega$. This mechanism is more efficient than resonant absorption for ${\mathrm{v}}_{\mathrm{osc}}/\omega >{\lambda }_g$ and the electron temperature scales as ${\mathrm{T}}_{\mathrm{hot}}\propto {\left(\mathrm{I}{\lambda }^2\right)}^{\alpha }$, where $\alpha >1$. For relativistic laser intensities and relatively large plasma gradients, $\mathrm{J}\times \mathrm{B}$ heating [23], arising from the oscillating component of the ponderomotive force, greatly dominates. The temperature of hot electrons resulting from this mechanism is of the order of the ponderomotive potential with a scaling of ${\mathrm{T}}_{\mathrm{hot}}\propto {\left(\mathrm{I}{\lambda }^2\right)}^{1/2}$ [24]. However, the effectiveness of this absorption mechanism is reduced when a high-density plasma with a sharp gradient is present [22].

As briefly presented above, the experimental conditions greatly affect the temperature of the energetic electrons and subsequently the accelerated protons in a very dynamic environment with no clear boundaries between different mechanisms. The experimental conditions can also vary between different laser systems of similar characteristics. In the following, we present and discuss our experimental findings on the influence of different laser polarization ($\mathrm{P},\mathrm{S}$, and ${45}^{°}$) on the number and energy of protons when varying laser intensity, pulse duration, and laser spot size are on the target.

2. Experiment

The experiments were carried out at the JETI40 laser facility at the Institute of Optics and Quantum Electronics at the University of Jena, Germany. The JETI40 laser system is based on chirped pulse amplification (CPA) technology with a center wavelength of $800\mathrm{nm}$ and can provide up to $650\mathrm{mJ}$ of pulse energy on target with a minimum pulse duration of $\sim 32\mathrm{fs}$ (FWHM). The pulse energy is monitored using a calibrated energy meter on a shot–shot basis. The polarization state of the laser was controlled by a 4-inch halfwave plate placed in the collimated beam before the focus. We considered the polarization state to be P- when the electric field component oscillates parallel to the plane of incidence, while S-polarized light oscillates perpendicularly to this plane. The laser pulses were focused using a ${45}^{°}$ (f/1.2) off-axis parabola (OAP) onto an aluminum target with a thickness of $6\mathsf{\mu }\mathrm{m}$. The focus spot size was $12\mathsf{\mu }{\mathrm{m}}^2$ at $(1/e^2)$, which accounts for an intensity above $1\times {10}^{19}\mathrm{W}/{\mathrm{cm}}^2$. The difference in reflectivity of the optics when changing the polarization state is about $1\%$, which is in the same range of shot–shot fluctuations. The energy spectra of the protons emitted in the target normal direction were measured by a single-shot Thomson parabola spectrometer (TPS) equipped with a microchannel plate (MCP) and a high-resolution charge-coupled device (CCD) (see Appendix A). The TPS has an acceptance angle of $2\mathsf{\mu }\mathrm{Sr}$ and is capable of detecting protons with energy from $30\mathrm{keV}$ up to several MeV in a single shot. We also used a calibrated electron spectrometer [25] based on magnetic deflection with image plates to measure the temperature of the electrons along the target normal direction. This spectrometer has an acceptance angle of $0.3\mathrm{mSr}$ and can measure up to several of tens of $\mathrm{MeV}$. A detailed schematic of the experimental set up is shown in Figure 1.

3. Results and Discussion

3.1. Intensity Scan

At first, we investigated the dependence of proton emission on laser intensity by varying the pulse energy on the target from $10\mathrm{mJ}$ up to $650\mathrm{mJ}$ in steps $<100\mathrm{mJ}$ while keeping the pulse duration and focus spot size fixed. We estimated the total number of protons collected by the TP for the energy range of $30\mathrm{keV}$ up to the maximum proton energy. In Figure 2a the integrated proton numbers for the three polarization states are presented. Error bars in all figures are due to shot–shot fluctuations. It can be seen that the total number of protons increases with laser intensity for all the polarization states. In fact, no significant difference can be observed in the proton number due to incident polarization, while the corresponding maximum proton energy presented in Figure 2b shows a clear preference for P-polarization state. To explain this observation, we take into account interaction parameters such as the intensity contrast ratio of the laser ∼${10}^{-6}$ at $10\mathrm{ps}$ and better than ${10}^{-10}$ at >$0.5\mathrm{ns}$. By taking a pre-plasma expansion velocity of ${\mathrm{c}}_{\mathrm{s}}\approx \sqrt{Z{k}_B{T}_e/m_i}$ with $Z=2$ as the charge state of aluminum atoms ionized at the pre-pulse, $k_B{T}_e<0.1\mathrm{keV}$ and $m_i$ is the ion atomic mass of aluminum; we found a pre-plasma scale length of $<0.4\lambda$. At high intensities for oblique incidencse (${45}^{°}$) of the laser pulse, P-polarization state has an electric field component directed parallel to the pre-plasma gradient $▽n$ at the reflection boundary, whereas for S-polarization this condition is not fulfilled [22]. Thus, for P-polarization, the non-collisional heating absorption mechanisms such as vacuum heating and resonance absorption are both greatly enhanced in comparison to the case when using S-polarized light.

Furthermore, we can also see that the maximum proton energy for P-polarized incident light follows a power-law of ($\mathrm{I}{\lambda }^2{)}^{\alpha }$ with $\alpha$ close to 1 for intensities up to $2.1\times {10}^{19}\mathrm{W}/{\mathrm{cm}}^2$. Thereafter, the power-law scaling reduces to $\alpha \sim 0.35$. We can infer that vacuum heating is the dominant mechanism for heating electrons in the plasma at low intensities [26], while with increasing intensities, resonance absorption contributes stronger [22]. For S-polarization, we see a similar trend but with lower proton energies, although the conditions for the parallel electric field vector are not optimized for vacuum and resonance heating. In fact, the measured scaling of $\alpha =0.38$ sits in between resonance absorption, $\alpha =0.3$ [22] and ponderomotive heating, $\alpha =0.5$ [21]. With this conclusion, we are not ignoring the fact that pondermotively accelerated electrons mainly follow the laser propagation direction. For our experiment, it is ${45}^{°}$, which we experimentally measured and presented in a previous work [27]. Here, the angle of emission is still energy-dependent [28] and for low energy electrons they have a wider spread, which covers the target normal direction. These observations agree to some extent with the theoretical work of Y. Sentoku [29].

As mentioned in the introduction, the maximum proton energy is proportional to the temperature of the hot-electron generation in the plasma ${\mathrm{E}}_{\mathrm{proton}}\approx \beta {\mathrm{T}}_{\mathrm{hot}}$. To quantify the factor $\beta$, we subsequently measured the temperature of the emitted electrons behind the target by inserting an electron spectrometer in the target normal direction (see Figure 1). The electron-energy spectra were taken at a maximum laser pulse energy of $650\mathrm{mJ}$. After applying a Maxwellian-like fit, we found an electron temperature of $T_P=0.46\mathrm{MeV}$ and $T_S=0.29\mathrm{MeV}$ for lasers with P-polarization and S-polarization states, respectively (Figure 3). This makes the factor ${\beta }_P\approx 4$ have good agreement with Y. Sentoku’s work [29]. For the S-polarization state, the factor is slightly higher ${\beta }_S\approx 4.1$.

3.2. Laser Pulse Duration Scan

Next, we fixed the laser energy at the maximum value and varied the temporal duration of the laser pulse and measured the corresponding maximum energy and number of protons. The scan range started from the optimized minimum pulse duration of $32\mathrm{fs}$ up to $180\mathrm{fs}$. We employed an acousto-optic programmable dispersive filter (AO-PDF), also called a Dazzler device, to vary the group delay dispersion [30]. We employed Spider and Wizzler devices [31] to measure the pulse duration for different Dazzler parameters. Pulse duration measurements were carried out routinely during the experimental period. This was achieved by coupling out the low power laser beam immediately onto the devices placed outside the interaction chamber using a fused silica window of $0.15\mathrm{mm}$ thickness and known dispersion, which allowed us to calculate the pulse duration in the interaction chamber. Although a fused silica glass wafer of $500\mathsf{\mu }\mathrm{m}$ thickness was employed to protect the gold parabola from target debris, the induced pulse elongation is less than $0.18\%$ [32].

Taking a look at the recorded maximum proton energy presented in Figure 4, we can see a slight energy increase followed by a general down-trend with increasing pulse duration. This behavior agrees with the work in [33]. As mentioned before, the intensity was not kept constant when varying the pulse duration, but only the energy, which was set at the maximum value of $650\mathrm{mJ}$. In the case of P-polarization—and less clearly in S and SP—we notice a maximum around $70–80\mathrm{fs}$. After this peak, however, the energy decreases with the laser pulse duration with a scaling law of ${(1/{\tau }_{\mathrm{laser}})}^{0.5}$. This is in agreement with the analytical model of a radially confined surface charge induced by laser-accelerated electrons on the target rear surface [34], as the laser energy ${\mathrm{E}}_{\mathrm{L}}={\mathrm{P}}_{\mathrm{L}}/{\tau }_{\mathrm{laser}}$ is converted with an efficiency of $\eta$ into hot-electron energy and subsequently into maximum proton energy as

$${\mathrm{E}}_{\max }=\alpha ·2{\mathrm{m}}_{\mathrm{e}}{\mathrm{c}}^2{\left(\eta \frac{{\mathrm{E}}_{\mathrm{L}}}{{\tau }_{\mathrm{laser}}·{\mathrm{P}}_{\mathrm{R}}}\right)}^{1/2}$$

(1)

where ${\mathrm{P}}_{\mathrm{R}}={\mathrm{mc}}^3/{\mathrm{r}}_{\mathrm{e}}$ is the relativistic power unit, ${\mathrm{r}}_{\mathrm{e}}$ is the classical electron radius, $\eta =0.4$ [35,36] is the conversion efficiency of energy transfer from laser into hot-electron, and ${\mathrm{E}}_{\mathrm{L}}$ and ${\tau }_{\mathrm{L}}$ are the laser energy and duration. We used a factor of $\alpha =0.22$ to obtain the same maximum proton energy of ${\mathrm{E}}_{\mathrm{p}}=2.3\mathrm{MeV}$, shown in Figure 4a at a pulse duration of ${\tau }_{\mathrm{laser}}=70\mathrm{fs}$. After substitution, the equation becomes equivalent to

$${\mathrm{E}}_{\max }=4.45\times {10}^{-20}\left[\mathrm{J}\right]·{\left(\frac{1}{{\tau }_{\mathrm{laser}}\left[\mathrm{s}\right]}\right)}^{0.5}$$

(2)

we used a quantity of $4.45\times {10}^{-20}\mathrm{J}$ in Equation (2) to fit the data in the case of P- and S-polarization states for the maximum proton energy after the peak at ${\tau }_{\mathrm{laser}}=70\mathrm{fs}$ and indeed we obtain a scaling of ${\left(\frac{1}{{\tau }_{\mathrm{laser}}}\right)}^{0.5}$.

On the other hand, when plotting the proton yield as a function of the laser pulse duration as seen in Figure 5, an uptrend is visible for all polarization states. The energy of the summed protons starts from the low energy threshold of the spectrometer $\sim 30\mathrm{keV}$ up to the maximum that is reported in Figure 4.

We compare our experimental findings with the theoretical estimation of the total number of protons given by the fluid model of Mora [37], and after some working we obtain

$${\mathrm{N}}_{\mathrm{p}}={\mathrm{n}}_{\mathrm{e}}{\mathrm{c}}_{\mathrm{s}}{\mathrm{t}}_{\mathrm{acc}}{\mathrm{S}}_{\mathrm{sheath}}·exp\left(-\sqrt{\frac{2\mathrm{E}}{{\mathrm{T}}_{\mathrm{hot}}}}\right){|}_{{\mathrm{E}}_{\max }}^{{\mathrm{E}}_{\min }}$$

(3)

where ${\mathrm{N}}_{\mathrm{p}}$ is the total number of accelerated protons over a given energy range, ${\mathrm{n}}_{\mathrm{e}}$ is the electron density, ${\mathrm{c}}_{\mathrm{s}}$ is the sound speed, ${\mathrm{t}}_{\mathrm{acc}}=\mathrm{a}·{\tau }_{\mathrm{laser}}$ is the acceleration time as discussed before [18] and ${\mathrm{S}}_{\mathrm{sheath}}$ is the sheath size at the target rear surface. We can see that the number of accelerated protons can increase with pulse duration as more electrons are involved in the light–energy conversion despite the lower maximum energy available for each particle. Using longer pulses can generate more protons; however, the acceleration time and the pulse energy are not infinite.

3.3. Laser Spot Size

In the next step, we fixed both the laser energy and the pulse duration while varying the laser spot size on the target. For that, we moved the target along the focus and as a result the intensity on the target varied with spot size ${\mathrm{w}}_{\mathrm{z}}$. We measured the maximum proton energy at each target position, as seen in Figure 6. The highest proton energy was recorded when using the P-polarized light and the lowest energy for the S-polarization of the incident light. Furthermore, for all polarization states the protons gain maximum energy at the focus corresponding to the highest intensity. Beyond the Rayleigh range, the energy drops off exponentially. A short variation in the maximum proton energy compared to Section 3.1 is seen, which we attribute to the shot–shot fluctuations.

When estimating the proton yield recorded at each focal position as presented in Figure 7, we can see a double-peak structure around the zero position of the focus. Indeed this feature is evident for all polarization states and can be accounted for by the volumetric effect. Although the laser intensity decreases fast away from the focus, the irradiated area on the target is larger, meaning that a higher number of particles is involved at a given volume. This, however, is only applicable if the intensity is still sufficient to generate hot electrons to go through the target and to accelerate the protons at the rear surface. To test that, we employed a Gaussian fit to the experimental peaks and found out that the average position of the peak in the case of P-polarization is around $\pm 155\mathsf{\mu }\mathrm{m}$ and slightly larger for the S-polarization state around $\pm 220\mathsf{\mu }\mathrm{m}$. Next, we calculated the equivalent intensity at this position assuming a Gaussian beam profile for the laser; ${\mathrm{w}}_{\mathrm{z}}={\mathrm{w}}_0\sqrt{1+{\left(\frac{\mathrm{z}}{{\mathrm{z}}_{\mathrm{R}}}\right)}^2}$ with $z_R=16\mathsf{\mu }\mathrm{m}$ is the Rayleigh length and ${\mathrm{w}}_0$ is the beam radius at the focus. This gives an intensity which is slightly lower than $1\times {10}^{18}\mathrm{W}/{\mathrm{cm}}^2$. At such intensity, we used the equation ${\mathrm{T}}_{\mathrm{hot}}=\kappa {\left(\mathrm{I}{\lambda }^2\right)}^{\alpha }$ to estimate the temperature of the electrons, with $\kappa$ being an experimental factor and $\alpha$ is a scaling factor which attributes the heating mechanism [38]. To set the factor $\kappa$, we used our experimentally measured value for the electron temperature of ${\mathrm{T}}_{\mathrm{hot}}=0.46\mathrm{MeV}$ at the minimum focal spot position and the scaling of $\alpha =0.35$. This gives $\kappa \approx 0.14$. Now we can estimate a temperature of ${\mathrm{T}}_{\mathrm{hot}}\approx 0.1\mathrm{MeV}$ when the target is placed at the peak position. These hot electrons still have to be involved in creating a strong enough sheath field to ionize and accelerate the protons at the target rear surface using a simple equation to estimate the electric field of the sheath at the exit behind the target ${\mathrm{E}}_{\mathrm{TNSA}}=\frac{\sqrt{2}{\mathrm{k}}_{\mathrm{B}}{\mathrm{T}}_{\mathrm{e}}}{e{\lambda }_D}$ [39], where ${\mathrm{k}}_{\mathrm{B}}{\mathrm{T}}_{\mathrm{e}}$ is the temperature of electrons and ${\lambda }_{\mathrm{D}}$ is Debye length. The (TNSA) electric field when the target is at the position where it gives the maximum proton number is $\sim 1\times {10}^{11}\mathrm{V}/\mathrm{m}$, which is about one order of magnitude lower than its value at the focus $\mathrm{z}=0$, yet it is still strong enough to ionize hydrogen atoms at the target side via barrier suppression of the atoms’ Coulomb field BSI [40] with a threshold electric field strength of ${\mathrm{E}}_{\mathrm{ion}}=\frac{\pi {ϵ}_0\ast ({\mathrm{U}}_{\mathrm{bind}}^2=13.6\mathrm{eV})}{e^3·(\mathrm{Z}=1)}\approx {10}^{10}\mathrm{V}/\mathrm{m}$.

In the case of S-polarization, we used our experimental scaling $\alpha =0.38$. By following a similar approach as in the case of P-polarization, we found that $\kappa =0.08$ and the reduced electron temperature $T_e=40\mathrm{keV}$, which corresponds to a sheath field of ${\mathrm{E}}_{\mathrm{TNSA}}=3\times {10}^{10}\mathrm{V}/\mathrm{m}$, to be compared to $\sim 7\times {10}^{11}\mathrm{V}/\mathrm{m}$ at the focus position.

To elaborate more on the two-peak feature seen in the proton yield, we tried to calculate the TNSA electric field and the interaction volume at different target positions. We started with the TNSA field, which, as discussed before, depends on the electron temperature $T_e$ and the Debye length ${\lambda }_D=\sqrt{\frac{{ϵ}_0{k}_B{T}_e}{e^2{n}_e}}$, where ${ϵ}_0$ is vacuum permittivity and $n_e$ the electron density at the target rear surface neglecting recirculation [39]. To estimate the electron temperature behind the target, we first calculated it at the target front surface at different target positions (which corresponds to different laser intensities), using the same simple scaling as before, $T_e\propto {\left(I{\lambda }^2\right)}^{0.35-0.38}$. These electrons are then injected into the target where their energy decreases mainly due to collisional energy transfer to bound atomic electrons following “Bethe” theory [41]. The TNSA field is then calculated for each target position. As expected, the TNSA electric field decreases as the electron temperature quickly declines away from the focus position. We also added a field ionization threshold limit of $\backsim {10}^{10}\mathrm{V}/\mathrm{m}$ for ionizing hydrogen atoms behind the target. The counteracting factor in our model is the increasing interaction volume of the incident laser pulse and the plasma created at the irradiated side of the target. We consider an interaction volume of $V_{inter}=\left(\pi w_z^2\right)·\left(t_{pre}{c}_s\right)$, where $\pi w_z^2$ is the focus spot size at the target and $t_{pre}=10\mathrm{ps}$ and $c_s$ are the pre-pulse time and pre-plasma expansion velocity, as introduced in Section 3.1. The product of $(E_{TNSA}·V_{inter})$, displayed in Figure 8, shows a similar behavior to the measured proton yield, especially when using the ionization limit of ${10}^{10}\mathrm{V}/\mathrm{m}$. It is worth mentioning that this simple model neglects some factors which are crucial for the laser–plasma interaction, for instance, the changing pre-plasma dynamics for different laser intensities as well as the interplay between different absorption mechanisms at different polarization states. To adequately tackle this task, however, extensive simulations are needed.

4. Conclusions

In summary, we have experimentally studied the effect of different laser parameters on the number and energy of accelerated protons during the interaction of high-intensity laser pulses with a thin aluminum foil. The total number of protons increased with laser intensity for all polarization states of the incident laser light. A slight saturation at intensities above $3\times {10}^{19}\mathrm{W}/{\mathrm{cm}}^2$ was also observed. A similar trend was also observed in the case of maximum proton energy. The measured scaling of maximum proton energy to electron temperature comes around $E_p\approx 4.1T_{hot}$, which agrees with theoretical work [29]. Further, we observed a slight increase in maximum proton energy when the laser pulse duration varied from $32\mathrm{fs}$ up to $70\mathrm{fs}$. The reported energy peak was followed by a decrease in maximum proton energy with increasing laser pulse duration for all polarization states. For P- and S-polarizations, we obtained a scaling of ${\mathrm{E}}_{\max }\sim {\left(\frac{1}{{\tau }_{\mathrm{laser}}}\right)}^{0.5}$. We also observed the uptrend of the total number of accelerated protons for longer laser pulses for all polarization states. Finally, we also varied the laser spot size on the target and observed the number of protons with respect to the spot size. We found a double peak structure away from the focus position for all polarization states due to the volumetric effect. It is important to carry out detailed parametric studies to understand the particle acceleration process for each laser system to find the optimal parameters for proton acceleration. Measuring the proton spectra along with the electron spectra enabled us to understand the dominating physical processes responsible for particle acceleration for the given laser parameters.