Plasma Emission from Dual Pulse Laser

Normally, double pulse LIBS (Singh & Thakur, Reference Singh and Thakur2007) uses two laser pulses separated by microsecond time delay. The first laser creates the plasma expanding normal to the target surface, whereas the second laser pulse gets absorbed in it followed by further ablation of target material by the residual second laser pulse. The absorption of second laser in the plasma created by the first laser pulse can be assumed to be dominated by inverse Bremsstrahlung absorption, which occurs due to electron — ion collisions in the plasma. If plasma electrons are subjected to momentum changing collisions as they oscillate back and forth in the laser electric field, the laser light wave undergoes an effective damping. The spatial damping rate of wave energy, k _ib can be given by (Max, Reference Max, Balian and Adams1982)

(1)$$k_{ib} \propto \displaystyle{{Zn_e^2 } \over {T_e^{3/2} \left({1 - \displaystyle{{n_e } \over {n_c }}} \right)^{1/2} }}.$$

Where n _e and T _e are the density and temperature of the plasma and Z is the atomic number of the target material. This shows that inverse Bremsstrahlung is strongest for the low temperature, high density, and high Z target materials. According to Eq. (1) a uniform plasma of length L and density n _e < n _c will produce a one way absorption fraction given by

(2)$${\rm \alpha} _{abs}=1 - \exp\left({ - k_{ib} L} \right).$$

For weak absorption k _ibL ≪  1 and α_abs ≅ k _ibL. For strong absorption, k _ibL ≫  1 and α_abs→1. This indicates that absorption fraction is linear in k _ibL for small absorption and then saturates when k _ibL is large. Even the long plasma length enhances the absorption. The result of inverse Bremsstrahlung absorption in inhomogeneous plasma is more complicated. A simplified version of absorption fraction for a linear density profile is given by (Max, Reference Max, Balian and Adams1982)

(3)$${\rm \alpha} _{abs}=1 - \exp \left\{{ - \displaystyle{{32} \over {15}}\displaystyle{{L{\rm \nu} _{ei} \lpar L\rpar } \over c}} \right\}\comma \;$$

where ν_ei (L) is the electron-ion collision frequency at critical density and c is the speed of light. This indicates that inverse Bremsstrahlung absorption is strongest for low temperature, high densities, high Z targets, and long density scale lengths. It is sensitive to details of the density profile near the critical surface and can be diminished considerably if the profile falls steeply at the critical surface. For simplification purpose, we have considered plasma expansion length L ≈ C _sT, where C _s is the ion acoustic (plasma expansion) speed and T is the plasma expansion time. An expression for the electron–ion collision frequency ν_ei can be given as (Bittencourt, Reference Bittencourt1986)

(4)$${\rm \nu}_{ei}=3.62\times10^{-6}n_{i} T_{e}^{-3/2} \ln\Lambda \; \; {\rm s}^{-1}.$$

where n _i (m⁻³) is the ion density in the plasma, T _e (K) is the plasma temperature and ln ∧ ~ 10. Electron-ion collision frequency ν_ei is considered to be the constant over the whole plasma length.

In the planar geometry, the volume of the radiating plasma can be approximately given by V= πR ²L for a plasma column of diameter 2R and length L. The mass ablated by the first and the second laser pulse can be given as m ₁πR ²τ_L and m ₂πR ²τ_L, respectively, where ṁ ₁ and ṁ ₂ are the mass ablation rate after the first and the second laser pulse, and τ_L is the time duration of both the lasers. The parameters of both the lasers are considered to be the same. It is well known that the plasma emission takes place through three processes, the Bremsstrahlung emission, the free-bound transition, and the bound-bound transition. In each case, the plasma emission is strongly dependent on the product of electron and ion density (∝ n _en _i), the temperature of plasma as well as on the volume of plasma. Considering that the plasma emission is proportional to the square of the plasma density (n _e = n _i) and the plasma volume, one can write an expression for the emission intensity after the first laser pulse (I ₁) as

(5)$$I_1 \propto \left({\displaystyle{{\dot m_1 {\rm \pi} R^2 {\rm \tau} _L } \over {{\rm \pi} R^2 C_{s1} T_1 }}} \right)^2 \left({{\rm \pi} R^2 C_{s1} T_1 } \right).$$

Where the first factor is the plasma density and the second factor is the volume of the plasma. C _s1 is the ion acoustic speed of the plasma due to first laser pulse and T ₁ is the time of plasma expansion that is gate delay from the first laser when the emission was recorded in single pulse LIBS.

The emission after the second laser pulse (I ₂) can be written as

(6)$$\eqalign { & I_2 \propto \left({\dot m_2 {\rm \pi} R^2 {\rm \tau} _L } \over {{\rm \pi} R^2 C_{s1} \Delta t+{\rm \pi} R^2 C_{s2} T_2 } \right)^2 \left({{\rm \pi} R^2 C_{s1} \Delta t+{\rm \pi} R^2 C_{s2} T_2 } \right)\cr & \qquad\times \left[{1 - \exp \left\{- {32 \over 15} {C_{s1} \Delta t{\rm \nu} _{ei} \over c}\right\}}\right].}$$

Here the first factor describes the plasma density after the time (Δt + T ₂), the second factor represents the plasma volume after the time (Δt + T ₂) and the third factor equals the fraction of the second laser absorbed in the plume of the plasma created by the first laser pulse. Δt is the time delay between the lasers, C _s2 describes the ion acoustic speed after the second laser pulse and T ₂ is the time (gate delay) after firing the second laser. To deduce a simplified expression for enhancement in double pulse emission and canceling all the common factors affecting the single and double pulse LIBS emission, the enhancement (E) is obtained by normalizing the sum of plasma emission under single and dual pulse LIBS by the emission from single pulse LIBS (Rai et al., Reference Rai, Yueh and Singh2008).

$${{I_1+I_2 } \over {I_1 }} =1+ {{I_2 } \over {I_1 }}\comma \;$$

(7)$$E = 1 + \left({\displaystyle{{\dot m_2 } \over {\dot m_1 }}} \right)^2 \displaystyle{{\left[{1 - \exp \left\{{ - \displaystyle{{32} \over {15}}\displaystyle{{C_{s1} \Delta t{\rm \nu} _{ei} } \over c}} \right\}} \right]} \over {\left({\displaystyle{{\Delta t} \over {T_1 }}+\displaystyle{{C_{s2} } \over {C_{s1} }}\displaystyle{{T_2 } \over {T_1 }}} \right)}}\comma \;$$

where one can take for the value of T ₁ any value between Δt (for maximum emission) and the time of peak emission in double pulse LIBS (from first laser pulse) without any significant change in the result. Eq. (7) has been used to study the effect of different parameters on the enhancement in plasma emission under dual pulse excitation, which explained various observations of dual pulse LIBS as reported earlier (Rai et al., Reference Rai, Yueh and Singh2008) . According to Eq. (7) zero delay between lasers (Δt = 0) provides an enhancement of unity (E = 1), just like a single pulse LIBS emission.

Plasma Emission from Single Pulse laser

Eq. (7) above obtained for dual pulse excitation of the plasma can be simplified for single pulse case under the light of above discussion that the plasma is formed and starts expanding when the initial portion of laser pulse interacts with the matter. So a single laser pulse can also be considered operating as dual pulse with certain assumptions. Mainly one can consider that after the plasma formation by pedestal of the laser, it expands for the period τ_L (duration of laser pulse) during which the laser gets absorbed in the expanding plasma. This indicates that Δt delay between two lasers in Eq. (7) can be replaced by τ_L for the single pulse case. Eq. (7) can be simplified in two ways as described below to better understand the dependence of important plasma parameters on the emission characteristics of the plasma as well as on its temporal behavior.

Case 1

In this case, assumption is made that the Δt = τ_L (laser time duration), T ₁ = τ_L/2 (time of peak laser intensity). T ₂ is the time at which the measurement of the plasma emission is taking place. Other consideration is that C _s2 = 2C _s1. In this situation, Eq. (7) can be written as

(8)$$E = 1+ \displaystyle{{\left({\displaystyle{{\dot m_2 } \over {\dot m_1 }}} \right)^2 \left[{1 - \exp \left\{{ - \displaystyle{{32} \over {15}}\displaystyle{{C_{s1} {\rm \tau} _L {\rm \nu} _{ei} } \over c}} \right\}} \right]} \over {\left({2+4\displaystyle{{T_2 } \over {{\rm \tau} _L }}} \right)}}.$$

This equation can provide information about the emission from the plasma at different time duration that means the variation of emission with the gate delay (T ₂).

Case 2

In this case, we consider Δt = τ_L and T ₁ = T ₂ = T is the gate delay or the time of measurement of the emission after the laser peak. Ratio of the laser pulse time duration τ_L and gate delay T (time of measurement) will be negligibly small for nanosecond time duration laser (τ_L/T ≈ 0). After these assumption Eq. (7) can be written as

(9)$$E = 1 + \left({\displaystyle{{\dot m_2 } \over {\dot m_1 }}} \right)^2 \left({\displaystyle{{C_{s1} } \over {C_{s2} }}} \right)\left[{1 - \exp \left\{{ - \displaystyle{{32} \over {15}}\displaystyle{{C_{s1} {\rm \tau} _L {\rm \nu} _{ei} } \over c}} \right\}} \right].$$

This indicates that the plasma emission under single pulse laser plasma interaction is mainly dependent on the square of the ratio of the mass ablation rate after full pulse and initial mass ablation, the ratio of plasma sound velocity, the plasma collision frequency and the pulse duration of laser.

Effect of Material Ablation

Figure 1 shows the variation in the emission intensity calculated theoretically using Eq. (9) for different values of the ratio of mass ablation rate of full laser pulse and its pedestal given as ${\dot m_2 } \over {\dot m_1 }$. For this calculation, ν_ei ~ 3.62 × 10¹² s⁻¹ is taken corresponding to a plasma density of 10¹⁷cm⁻³ and a plasma temperature of 1 eV. The ratio of plasma sound velocity of full intensity plasma and initial (pedestal) plasma is kept as ${C_{s2} \over C_{s1}} { \sim \!\!2}$. The variation has been shown for 1, 10, and 20 ns laser pulses. The variation shows that the emission intensity increases as the value of ${\dot m_2 } \over {\dot m_1 }$ increases. Initially, increase in emission intensity is slow but for the higher value of ratio of mass ablation rates, it increases fast as emission is proportional to the square of ratio of mass ablation rates. Normally, material ablation is directly related with the laser intensity, which indicates that ultimately an increase in the laser intensity increases the plasma emission. The time duration of the laser pulse also plays an important role in plasma emission as emission intensity increases with an increase in the time duration of laser. These observations are as expected because an increase in interaction time keeps the plasma hot for a longer time as a result of efficient absorption of the laser providing more emission from the plasma. These results are in agreement with the experimental observations reported earlier (Zeng et al., Reference Zeng, Mao, Grief and Russo2005; Leitz et al., Reference Leitz, Redlingshofer, Reg, Otto and Schmidt2011).

Fig. 1.

(colour online) Variation in emission intensity from plasma with change in ratio of mass ablation rate $\displaystyle\lpar{{\dot m_2 } \over {\dot m_1 }}\rpar$ for plasma produced by 1, 10, and 20 ns time duration laser.

It is well known that many parameters decide about the initial ablation of sample material by pedestal of the laser at very low intensity (Piepmeier, Reference Piepmeier and Piepmeier1986). These parameters, such as sample reflectivity, thermal conductivity, vaporization temperature, heat capacity and latent heats of fusion, and vaporization, are important in determining the total amount of material removed from the sample. At starting of the laser pulse, electrons and ions are released from the surface by photoelectric and thermionic processes. The free electrons above the surface gain energy by absorbing photons from the laser beam. This initial plasma may trigger the generation of more plasma that is formed by thermal ionization of the vaporizing bulk material of the sample. Initially, at lower irradiances, the sample material at the surface is not heated much above its boiling temperatures. In this case, velocity of the vaporizing materials is on the order of ~ 10⁴ cm s⁻¹. However, at higher irradiances the velocities of the sample species reach values above 10⁶ cm s⁻¹ corresponding to the particles with energies above their normal boiling temperatures (Piepmeier, Reference Piepmeier and Piepmeier1986). In this situation, X-rays and highly ionized species are also observed indicating that energies of the plasma reached from ten to hundreds of electron volts, which comes down after expansion. Individual particles of high energy result from the highly energetic plasma generated by inverse Bremsstrahlung absorption of the high power density of laser beam. The amount of material ablated depends on the time duration of the laser. It is several orders of magnitude lesser for short time duration laser (Piepmeier, Reference Piepmeier and Piepmeier1986, Zeng et al., Reference Zeng, Mao, Grief and Russo2005; Leitz et al., Reference Leitz, Redlingshofer, Reg, Otto and Schmidt2011). This is because much shorter time is available for conduction of heat into the sample. This indicates that energy of the shorter laser pulse is therefore useful in processes near the surface rather than in vaporizing material at greater depth. Crater depth in material ranges from 1 to 10 µm for a Q switched laser and the amount of material ablated is generally at and below the microgram level (Piepmeier Reference Piepmeier and Piepmeier1986). A comparison shows that short pulse micro and nanosecond laser systems generally allow high ablation rates, where the possibility of thermal damage of the target piece is higher. On the other hand ultrafast picosecond and femtosecond laser systems provide lower ablation efficiency but allow a higher precision in ablation (Leitz et al., Reference Leitz, Redlingshofer, Reg, Otto and Schmidt2011).

Effect of Plasma Density (Laser Energy)

It is well known that during laser matter interaction an increase in laser intensity increases the plasma density as well as plasma temperature. Plasma density increases due to increased material ablation, whereas plasma temperature increases due to absorption of laser energy into plasma preformed due to pedestal (initial part) of the laser. To better understand the effect of plasma density and temperature on the process of plasma emission, calculation was made using Eq. (9) for different values of electron-ion collision frequencies, because it is decided by the value of plasma density and temperature. Ultimately, this collision frequency plays an important role in absorption of laser energy into plasma. For this calculation, we took ${\dot m_2 \over {\dot m_1 }} = 4$ and ${C_{s2} \over C_{s1}} = 2$Figure 2 shows the variation in emission intensity with an increase in plasma density (10¹³ to 10²⁰ cm⁻³) for different values of plasma temperature (1, 5, and 10 eV). It shows that initially plasma emission increases slowly followed by a fast nearly linear increase in emission between 10¹⁵ to 10¹⁹ cm⁻³. However, a further increase in plasma density beyond 10¹⁹ cm⁻³ shows saturation in emission. It has been noted that the emission intensity is high for lower value of plasma temperature, which is expected as the value of electron-ion collision frequency remains high for low plasma temperature. This increases the absorption of the laser intensity by the plasma, which results in a stronger emission. Another observation is that emission intensity starts increasing and saturating at comparatively lower-value of plasma density for low temperature plasma. Again the role of plasma frequency is found to be more important. Finally, one can say that an increase in laser intensity increases the plasma density as well as the temperature, where the balance between the two effects leads towards saturation in emission.

Fig. 2.

(colour online) Variation in emission intensity with an increase in plasma density for plasma temperature of 1, 5, and 10 eV.

It is important to compare the results of this calculation with the experimental observations. Rai et al. (Reference Rai, Rai, Yueh and Singh2003b) has reported the effect of laser energy on the LIBS signal in the presence of magnetic field. LIBS spectra of aluminum alloy sample were recorded in the absence as well as in the presence of a magnetic field, where the energy of the laser was varied from 10–150 mJ (4 × 10⁹–60 × 10⁹ W/cm²). The variation of chromium line intensity (l = 357.87 nm) with laser energy in the absence of a magnetic field shows that emission intensity increases first very slowly and then very fast up to nearly 20 mJ. Further increase in laser energy saturates the chromium line emission intensity. It seems that initially the laser radiation is absorbed up to 20 mJ, where ablation of the material and consequently density of plasma increases with laser intensity and gets saturated. These observations are similar as obtained by theoretical calculations (Figs. 1 and 2). However, the excess laser energy beyond 20 mJ (≥8 × 10⁹ W/cm²) is not being coupled (absorbed) to laser produced plasma. This is possible only due to shielding produced by the plasma near critical density (10²¹ cm⁻³) surface formed at high laser intensity where electron-ion collision frequency is >10¹³ s⁻¹. Similar behavior of plasma emission has been reported (Aguilera et al., Reference Aguilera, Aragon and Penalba1998). Probably excess laser energy is being reflected from the critical density surface of the plasma, where the plasma frequency becomes equal to the laser frequency. In this case, laser can not propagate toward the higher plasma density side. At higher plasma density, self-absorption of emission is also possible leading to saturation, when the experiment is performed at higher laser intensity. The presence of self-absorption can be observed from the measurement of full width at half maximum of the Lorenzian profile of line emission (Aguilera et al., Reference Aguilera, Aragon and Penalba1998). Both the processes are possible in the high density plasma, which can contribute toward saturation (or decrease in saturation) in the emission. The breakdown in gases surrounding the target also shields the laser energy reaching the target surface, which results in decrease and/or saturation in material ablation from the target surface and consequently in the plasma emission (Batani, Reference Batani2010; Lee et al., Reference Lee, Kim, Jung and Yun2011). Rai et al. (Reference Rai, Rai, Yueh and Singh2003b) further report that the presence of magnetic field shows no significant effect on atomic line emission intensity, when the laser energy was below 10 mJ (when the plasma density is low). However, an increase in the emission intensity in the presence of a magnetic field was noted for laser energy between 10 to 50 mJ. This enhancement in emission in the presence of magnetic field is due to an increase in the plasma density (electron-ion collision frequency) as a result of magnetic confinement of the plasma, which is effective at lower plasma temperature, when the laser intensity is lower. However, this enhancement in emission intensity decreased, when the laser energy was further increased beyond 50 mJ. The plasma emission in the presence of a magnetic field was even lower than the emission observed in the absence of a magnetic field for laser energy >80 mJ (32 × 10⁹ W/cm²). It seems that along with reflection of laser energy from critical density level and self-absorption of emission, some other loss factors are also added up in the presence of magnetic field. This extra factor may be due to the presence of density fluctuation (instability) in the plasma, which is generated at higher laser intensity in the presence of a magnetic field. Density fluctuations are expected in this situation due to bouncing of the plasma near β = 1 location, where plasma kinetic energy becomes equal to the magnetic energy. Even some high-frequency instability, such as large Larmor radius instability is also expected in such plasma condition (Cabalin & Laserna, Reference Cabalin and Laserna1998; Rai et al., Reference Rai, Rai, Yueh and Singh2003b). The presence of instability in the plasma can lead to the scattering of laser light as well as the loss of plasma particles as a result of cross field diffusion. This may be the reason behind the decrease in emission intensity even after saturation, when the laser energy is more than 80 mJ in the presence of magnetic field. Similar behavior is noted for iron line emission at λ = 358.12 nm with an increase in laser energy in the absence and presence of magnetic field.

In another plasma experiment (Rai et al., Reference Rai, Singh, Fang and Cook2003c), the plasma is formed from liquid jet target having magnesium in low concentration. It is noted that the intensity of all three magnesium lines increases linearly with laser energy up to ~ 300 mJ in the absence of magnetic field. But the presence of the magnetic field shows an enhancement in the LIBS intensity up to 200 mJ, followed by a saturation/decrease toward higher laser energy. The maximum signal enhancement was observed between 150–200 mJ of laser energy. Similar enhancement in the emission intensity was noted for other elements also such as Magnesium, chromium, and titanium in aqueous solution in the presence of magnetic field. Although the threshold laser energy for the breakdown was ~ 10 mJ for solid sample in comparison to ~ 50 mJ for a liquid sample, even then the basic observations are similar for solid or liquid samples. The enhancement in the emission intensity was noted mainly for moderate laser energy after the breakdown. Finally, these experimental observations are found in agreement with the theoretical calculations.

Saturation in Plasma Emission

The study of variations in plasma emission with electron density and temperature for laser of different time duration can provide better understanding of saturation in plasma emission. For this purpose, the calculation is performed using Eq. (9) with a consideration that ${\dot {m_2} \over \dot {m_1}} = 4$, ${C_{s2} \over {C_s1} } = 2$ and T_e = 1eV and the results are presented in Figure 3, which shows the variation in plasma emission with change in plasma density for different time duration of the laser τ_L. It is shown that the plasma emission starts increasing at ~ 10¹⁶ cm⁻³ for a laser of 1 ns time duration. This increase became fast with an increase in plasma density, which saturates at ~10¹⁹ cm⁻³. Similar variations are noted for 10 and 20 ns time duration laser, but with minor change in the threshold for initiation and saturation of emission, which occur at lower density for large time duration lasers. Higher time duration laser produce comparatively more plasma emission as a result of more material ablation (Zeng et al., Reference Zeng, Mao, Grief and Russo2005; Leitz et al., Reference Leitz, Redlingshofer, Reg, Otto and Schmidt2011). Here again the electron-ion collision frequency and laser plasma interaction time play an important role. In this case, the plasma collision frequency increases with an increase in the plasma density, which helps in increasing the absorption of laser in plasma through inverse Bremsstrahlung and consequently the plasma emission, whereas large time duration of laser provides longer time for plasma to expand and absorb the laser efficiently.

Fig. 3.

(colour online) Variation in emission intensity with an increase in plasma density for plasma produced by 1, 10, and 20 ns time duration laser.

The effect of plasma temperature on its emission has also been obtained using Eq. (9), where the plasma density was constant at ~ 10¹⁷ cm⁻³ keeping all other parameters the same as in Figure 3. In this case, emission from plasma is calculated by varying the plasma temperature for different time duration laser. Figure 4 shows that plasma emission is very high for low temperature plasma, which decreases first very fast and then slowly with an increase in plasma temperature. The reason for decrease in plasma emission with an increase in plasma temperature is due to decrease in electron-ion collision frequency as ν_ei ∝ (T _e)^−3/2. Here again plasma emission is high for longer time duration laser as seen in earlier case. In this case, saturation is seen at lower plasma temperature near 1 eV. Results of Figures 3 and 4 indicate that saturation in the plasma emission is possible only when the plasma density is high and plasma temperature is low. In other words, one can say that instead of plasma density and plasma temperature, electron-ion collision frequency play an important role in deciding the saturation in plasma emission, which is ν_ei > 10¹³ s⁻¹ as has been discussed earlier.

Fig. 4.

(colour online) Variation in emission intensity with an increase in plasma temperature for plasma produced by 1, 10, and 20 ns time duration laser.

Laser Absorption and Shielding Effect in Plasma

The observation of figures 1 and 2 can be better understood by considering variation in the laser absorption mechanism with an increase in laser intensity. For lower laser intensity, a laser-supported detonation wave is expected in which the laser absorption region propagates as a shock wave (Aguilera et al., Reference Aguilera, Aragon and Penalba1998). In this regime, if the electron density remains below the critical density then an increase in laser intensity will increase its absorption in the plasma resulting in more ablation as well as plasma emission. This is the reason why plasma emission increases linearly with laser intensity. When the plasma density reaches critical density level, the plasma becomes opaque to the laser beam, which shields the target. In this case, coupling of laser intensity to plasma decreases, which lead to a saturation in plasma emission. This phenomenon can be observed in both types of targets (solid and liquid) when the laser intensity is in the medium range. This saturation takes place at comparatively low laser intensity for solid in comparison to liquid sample due to production of higher plasma density in the case of solid targets. At higher laser intensity, the absorption mechanism changes to laser- supported radiation wave, in which plasma temperature becomes very high resulting in transparent plasma for the laser beam, which starts emitting Bremsstrahlung (background) emission due to its high temperature (Aguilera et al., Reference Aguilera, Aragon and Penalba1998). The plasma shielding effect is then reduced and the ablation of the target material enhanced. In this regime also, plasma emission (X-rays and visible) intensity increases linearly. Saturation in the X-ray emission was also noticed in the form of change in the slope with an increase in the laser intensity. However, this saturation was found to be correlated with the loss of plasma energy in form of the generation of instability and high energy particles in the plasma along with emission of high energy X-rays (Rai et al., Reference Rai, Shukla and Pant2000a, Reference Rai, Shukla and Pant2000b). Normally, the high-intensity laser experiment involves measurement of X-ray emission under vacuum conditions. However, the high laser intensity experiment in air also shows saturation, where the shielding of the laser occurs by the air plasma (Aguilera et al., Reference Aguilera, Aragon and Penalba1998; Lee et al., Reference Lee, Kim, Jung and Yun2011). In this case, presence of the target surface enhances breakdown in the surrounding gas, which is why air plasma is also formed when the laser is focused below or on the sample surface (Multari et al., Reference Multari, Foster, Cremers and Ferris1996).

Temporal Evolution of Emission from Confined Plasma

The temporal evolution of plasma emission is obtained using Eq. (8). For this purpose, we have considered T ₁ = τ_L/2 (Peak time of laser) and T ₂ is varied, which is equivalent to the time delay at which the emission intensity is recorded. To see the effect of plasma confinement and the laser time duration on the temporal evolution, calculations have been performed first for different values of C _s2/C _s1 as 2, 0.5, and 0.1 keeping laser time duration constant at 10 ns and then for 1, 10, and 20 ns time duration laser keeping C _s2/C _s1 constant at ~ 2. Figure 6 has the variation of plasma emission with time delay for decreasing value of C _s2/C _s1, which shows plasma confinement effect. It shows that for C _s2/C _s1~ 2 plasma emission first decreases very fast and then slowly with time delay. After adding the confinement effect by decreasing the values of C _s2/C _s1 to 0.5 and 0.1, plasma emission increases for all the delay time. Even the rate of decay in emission intensity changes, which indicates that plasma emission last for a longer time in the case of plasma confinement. It further shows that maximum enhancement in the emission after confinement occurs around the time delay of 20 ns. This happens because of slowing down of decay in plasma emission as a result of plasma confinement. Figure 7 shows the variation in temporal evolution of plasma emission obtained from a laser having time duration of 1, 10, and 20 ns. Here the plasma emission is less for 1 ns laser produced plasma, which initially decays fast and then slowly. The rate of plasma decay decreases with an increase in time duration of the laser. Even the emission is higher for the plasma produced by a longer time duration laser, which is due to efficient heating of the plasma for a longer time as discussed earlier. It also shows that plasma produced by a long time duration laser lasts for a longer time. These observations are in agreement with the experimental observations (Zeng et al., Reference Zeng, Mao, Grief and Russo2005; Leitz et al., Reference Leitz, Redlingshofer, Reg, Otto and Schmidt2011).

Fig. 6.

(colour online) Variation in emission intensity with time of measurement after laser peak for plasma having ratio of expansion velocity (C _s2/C _s1) as 0.1, 0.5, and 2.

Fig. 7.

(colour online) Variation in emission intensity with time of measurement after laser peak for plasma produced by a laser of 1, 5, and 10 ns time duration.

Similar observation has been reported experimentally (Rai et al., Reference Rai, Rai, Yueh and Singh2003b). They have studied temporal evolution of chromium line emission from aluminum alloy in the absence and presence of a magnetic field (magnetic confinement) and reported that plasma emission was maximum at ~ 2 μs after which it started decreasing. The emission intensity lasted for nearly 20 μs. An overall increase in intensity was noted for all the delay in the presence of magnetic field (magnetic confinement), whereas the shape of the curve remained the same. This result is similar as shown in Figure 6. The decay in emission with time indicates that initially the plasma is hot and the emission from it is dominated by the background emission, which contains mainly Bremsstrahlung emission. As the gate delay increases, the plasma expands away from the target and gets cool resulting in a decrease in emission. The presence of the magnetic field increases the effective density of plasma in the emission volume as a result of confinement of laser produced plasma, which ultimately increases the probability of radiative recombination, electron-ion collision frequency as well as absorbed energy per unit volume. All of these factors play role in increasing the plasma emission.

During magnetic confinement enhancement in plasma emission and deceleration in plasma expansion changes with plasma β (Rai et al., Reference Rai, Rai, Yueh and Singh2003b). It is well known that plasma β depends mainly on the density and temperature of the plasma, which decreases as the plasma expands away from the target. It also depends on the intensity of magnetic field, which remains constant during this experiment. It is shown that initially for a higher value of β, the plasma deceleration and enhancement in emission is negligible. However, as the β decreases below 10, the ratio of plasma expansion velocities v ₂/v ₁ decreases and the ratio of emission intensity I ₂/I ₁ (value of enhancement) increases. This indicates that Bremsstrahlung emission, which occurs at higher plasma temperatures and density (β > 10) and comparatively at early time (smaller gate delay) after the plasma formation, cannot contribute to the enhancement in the emission. Mainly line emissions are getting affected due to recombination radiations or heating of plasma as a result of its confinement. These reported results are also in qualitative agreement with the theoretical findings of this paper.